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Q: Function of aapt/AndroidManifest.xml in AAR Some of my Android libraries (AAR files) contain an aapt/AndroidManifest.xml as well as the root AndroidManifest.xml. From what I could see, these two don't differ, but the one in aapt seems to be optional. I couldn't find any documentation about it though. So what's the purpose of this second manifest? And why is it added only sometimes? A: @NonNull @Override public File getAaptFriendlyManifestOutputFile() { return FileUtils.join( globalScope.getIntermediatesDir(), "manifests", "aapt", getVariantConfiguration().getDirName(), "AndroidManifest.xml"); }	{ "pile_set_name": "StackExchange" }
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The Ultimate Guide for Alternative Brides Rockstar Vendor Tobi Hannah Occasionwear A/W 2011 The very lovely Tobi Hannah launches her A/W 2011 occasionwear this month and I’m thrilled to share the key pieces in the new collection with you. The core pieces are all black, bright pink or royal blue…all my favourite colours! The structured designs are bang on trend (I kinda hate that I just used that phrase but it is true…) and each piece is inspired the work of British sculptor, Jeff Lowe. I just love them all but I’m particularly drawn to Andi (love that skirt), Audrey (love the shape) and Olive (cute cute cute!) You?	{ "pile_set_name": "Pile-CC" }
All alone, Yellow Guy tries to stop a lamp from teaching him about dreams. While Red Guy finds out the truth about the puppet's existence.	{ "pile_set_name": "OpenWebText2" }
--- abstract: 'We derive an $S=1$ spin polaron model which describes the motion of a single hole introduced into the $S=1$ spin antiferromagnetic ground state of Ca$_2$RuO$_4$. We solve the model using the self-consistent Born approximation and show that its hole spectral function qualitatively agrees with the experimentally observed high-binding energy part of the Ca$_2$RuO$_4$ photoemission spectrum. We explain the observed peculiarities of the photoemission spectrum by linking them to two anisotropies present in the employed model—the spin anisotropy and the hopping anisotropy. We verify that these anisotropies, and not the possible differences between the ruthenate ($S=1$) and the cuprate ($S=1/2$) spin polaron models, are responsible for the strong qualitative differences between the photoemission spectrum of Ca$_2$RuO$_4$ and of the undoped cuprates.' author: - 'Adam Kł‚osiń„ski' - 'Dmitri V. Efremov' - Jeroen van den Brink - Krzysztof Wohlfeld date: - - title: \| Photoemission Spectrum of Ca$_2$RuO$_4$:\ Spin Polaron Physics in an $S=1$ Antiferromagnet with Anisotropies --- Introduction. {#sec:introduction} ============= Understanding the strongly correlated physics of the transition metal oxides constitutes a nontrivial task [@Dagotto1994; @Imada1998; @Lee2006; @Khomskii2010; @Khomskii2014]. On one hand, this is due to the fact that even the simplest, but still realistic, effective models may have to contain several degrees of freedom. On the other, this is due to the fact that such relatively simple models are often not solvable in the thermodynamic limit. That is why examples when a theoretical model can be solved without too drastic approximations [and]{} explain the experimentally observed features of a correlated oxide are of interest. One such case, known already since the end of the 80s of the last century, is the so-called spin polaron problem [@Schmitt1988; @Martinez1991; @Ramsak1998; @Manousakis2007; @Wang2015; @Grusdt2018; @Bieniasz2019], which explains the peak dispersion found in the photoemission spectrum of the (spin $S=1/2$) antiferromagnetically ordered and Mott insulating copper oxides [@Wells1995; @LaRosa1997; @Kim1998; @Damascelli2003; @Shen2007]: It turns out that the peak dispersion found in the spectra of the ‘parent compounds’ to the high-temperature superconductors can be well explained using a $t$–$J$ or Hubbard model that is mapped onto a (spin) polaron problem. Interestingly, despite the still unresolved mysteries associated with high-temperature superconductivity, the copper oxides are the simplest class of oxides to model. This is basically due to the fact that the uncorrelated part of their physics can be effectively described using a single-band picture [@Zhang1988; @Lee2006]. Such situation is not realised in many other oxides, such as the manganites, vanadates, nickelates—or the ruthenates studied here [@Imada1998; @Khomskii2014]. In this case the effective models are far more involved and are never of the single-band $t$–$J$ or Hubbard variety. Can one thus expect that some of the principles of the spin polaron physics do hold there? To investigate this rather general problem, we take a closer look at one of the intensively investigated transition metal oxides—Ca$_2$RuO$_4$ [@Alexander1999; @Nakatsuji2000; @Mizokawa2001; @Lee2002; @Gorelov2010; @Kunkemoeller2015; @Fatuzzo2015; @Kunkemoeller2017; @Jain2017; @Sutter2017; @Zhang2017; @Das2018; @Ricco2018; @Pincini2019; @Gretarsson2019] which is a spin $S=1$ antiferromagnetically ordered [@Mizokawa2001; @Kunkemoeller2015; @Kunkemoeller2017; @Das2018; @Pincini2019] and Mott insulating analogue of the unconventional superconductor Sr$_2$RuO$_4$ [@Maeno1994]. The other reason for choosing this system is that recently its detailed photoemission spectrum was not only studied experimentally but also successfully modelled using a multiband Hubbard model [@Sutter2017]. Nevertheless, as the multiband Hubbard model was solved using the single-site dynamical mean-field theory approach, it is not clear to what extent the spin polaron physics is present there. In this paper we concentrate on the origin of the incoherent and almost momentum-independent Ca$_2$RuO$_4$ photoemission spectrum, that is present at the high-binding energy part \[see the yellow rectangle of Fig. \[result\](a)\] and is associated with the hole motion in the $xz$ and $yz$ orbitals [@Sutter2017]. The reason for leaving the $xy$ orbital out of our analysis is that the highly dispersive, quasiparticle-like part of the photoemission spectrum stretching from low- to high-binding energy \[see Fig. \[result\](a)\] can be easily understood as the free hole motion on the $xy$ orbitals. This follows straightforwardly from, on the one hand, the relatively large energy gap between the $xy$ and $xz/yz$ orbitals leading to the $xy$ orbital being fully occupied and, on the other hand, the absence of any mixing between $xy$ and $xz/yz$ orbitals, be it from hopping or the Coulomb interaction. Thus, including the $xy$ orbitals in our analysis would not much enrich our understanding of the physics at work in this compound. Altogether, our aim here is twofold: First, we want to model the high-binding energy part of the photoemission spectrum of Ca$_2$RuO$_4$ by using a realistic [$S=1$ spin polaron]{} model, specifically derived for this case. Second, we wish to understand to what extent such an $S=1$ spin polaron problem is different from the ‘standard’ (i.e. $S=1/2$) spin polaron model that is well-known from the cuprate studies. The paper is organized as follows. In Sec. \[sec:tjmodel\] we introduce the $t$-$J$ model that describes the motion of a single hole in the ground state of Ca$_2$RuO$_4$. Next, in Sec. \[sec:fromto\] we perform a mapping of the $t$-$J$ model onto a S=1 spin polaron model. The latter is solved using the self-consistent Born approximation (SCBA) in Sec. \[sec:mandr\]. Finally, we discuss the obtained results in Sec. \[sec:discussion\] and end the paper with conclusions in Sec. \[sec:conclusions\]. The paper is supplemented by an Appendix which contains some details of the mapping from the $t$-$J$ to the polaron model. ![Comparison between the experimental and theoretical spectral functions of Ca$_2$RuO$_4$: (a) Angle resolved photoemission (ARPES) spectrum obtained for Ca$_2$RuO$_4$ and published in Ref. ; (b) Hole spectral function $A({\bf k}, \omega)$ calculated for the spin $S=1$ $t$–$J$ Hamiltonian (\[model1\]-\[model2\]) with ${\bf e}_{xz} = \hat{x}$, ${\bf e}_{yz}=\hat{y}$ and using the mapping onto the spin-polaronic model (\[finalhamiltonian\]) and the SCBA method (see text); model (\[finalhamiltonian\]) parameters: $t = 22 J$, $\epsilon = 5.6 J$, $\gamma = 0.25 J$, $J = 5.6 $ meV, numerical broadening of $A({\bf k}, \omega)$ $\delta = 1.1 J $; (c) Hole spectral function $A({\bf k}, \omega)$ calculated as in (b) but convoluted with a Gaussian with the half-width at half maximum equal to $0.5t$, simulating the experimental resolution of ARPES on Ca$_2$RuO$_4$ [@Sutter2017]. The yellow rectangles mark the high binding energy parts of the spectra that are incoherent and almost momentum-independent, are identified in ARPES as having a dominant $xz$/$yz$ orbital character [@Sutter2017], and are theoretically modelled by panel (b) \[The dispersive branch visible in (a), both inside and outside of the yellow rectangle and not discussed here, is associated with the $xy$ orbital [@Sutter2017]. See main text of the paper\]. Theoretical spectra (b-c) are normalised in the same manner as the ARPES spectrum \[(a)\] of Ref. . []{data-label="result"}](fig1.png){width="50.00000%"} ${\bf t}$-${\bf J}$ model. {#sec:tjmodel} ========================== In order to model (the high-binding energy part of) the photoemission spectrum of Ca$_2$RuO$_4$ we follow the scheme that was already developed ca. 30 years ago and, as mentioned in the introduction, was successfully used to describe, [inter alia]{}, the photoemission spectra of several undoped copper oxides [@Wells1995; @LaRosa1997; @Kim1998; @Damascelli2003; @Shen2007]. Thus, we consider an appropriate $t$–$J$-like Hamiltonian constructed as a sum of two parts ${\mathcal H} = {\mathcal H}_J+ {\mathcal H}_t$. The first part, ${\mathcal H}_J$, describes the low energy physics of the Mott insulating Ca$_2$RuO$_4$ in terms of the interaction between the localised $S=1$ magnetic moments. The relevant Hamiltonian is well-known in this case and reads [@Kunkemoeller2015; @Kunkemoeller2017; @Jain2017], $$\label{model1} {\mathcal H}_J = J \sum\limits_{\langle {\bf i}, {\bf j} \rangle} \mathbf{S_{\bf i}} \cdot \mathbf{S_{\bf j}} + \epsilon \sum\limits_{\bf i} \left( S_{\bf i}^z \right)^2 + \gamma \sum\limits_{\bf i} \left( S_{\bf i}^x \right)^2,$$ where the summation runs over all nearest-neighbour pairs on a 2D square lattice, $J$ is the spin exchange constant, and $\mathbf{S_{\bf i}}$ are the spin $S=1$ operators. As already discussed in Refs. the spin model is highly anisotropic, with the suggested values of the $\hat{z}$ ($\hat{x}$) axis anisotropy being equal to $\epsilon = 5.6 J$ ($\gamma = 0.25 J$), respectively, with $J = 5.6$ meV reproducing the spin wave dispersion observed in the inelastic neutron scattering experiment [@Kunkemoeller2015; @Kunkemoeller2017; @Jain2017]. We note that such a large spin anisotropy originates in the large spin-orbit coupling on the ruthenium ions which, however, is quite widely considered as not strong enough to stabilise the $S=0$ ground state [@Mizokawa2001; @Kunkemoeller2015; @Kunkemoeller2017; @Das2018; @Pincini2019]. Although the latter result can naively be understood as a consequence of the crystal field splitting (between the $xz, yz$ and the $xy$ orbitals) being about twice larger than the spin-orbit coupling [@Das2018] and therefore the spin $S=0$ states having considerably higher energy than the spin $S=1$ states, see Fig. S1 of [@Jain2017], it has been postulated [@Khaliullin2013; @Akbari2014; @Jain2017; @Gretarsson2019] that nevertheless the ‘excitonic magnetism’ can be at play here. The second part of the Hamiltonian, ${\mathcal H}_t$, is the ‘kinetic’ term. This term is introduced, in order to describe the motion of a single hole created in the ruthenium oxide plane in the photoemission experiment. We restrict our model to the $xz$ and $yz$ orbitals, for, as discussed in the introduction, we are solely interested in the part of the photoemission spectrum associated with these orbitals [@Sutter2017]. Altogether, we end up with, $$\begin{aligned} \label{model2} \begin{split} {\mathcal H}_t &= - t \sum\limits_{{\bf i}, \sigma} \left( \tilde{c}_{{\bf i}+{{{\bf e}_{xz}}},xz,\sigma}^{\dag} \tilde{c}_{{\bf i},xz,\sigma} +\tilde{c}_{{\bf i}+{{\bf e}_{yz}},yz,\sigma}^{\dag} \tilde{c}_{{\bf i},yz,\sigma} +h.c.\right),\\ \end{split}\end{aligned}$$ where the first (second) term describes the hoppings of an electron with spin $\sigma$ between the nearest neighbor ruthenium $xz$ ($yz$) orbitals along the ${\bf e}_{xz}=\hat{x}$ (${\bf e}_{yz}=\hat{y}$) direction in the 2D square lattice, respectively. Such effectively one-dimensional (‘directional’) hoppings follow from the Slater-Koster scheme [@Slater1954] applied to the square lattice geometry of the ruthenium oxide plane and is, in fact, a common feature of systems with active $\{xz, yz\}$ orbital degrees of freedom [@Harris2004]. As for the value of the hopping element $t$ in Ca$_2$RuO$_4$ we choose $t= 123$ meV [@Gorelov2010], i.e. $t = 22J$ for the above chosen realistic value of $J=5.6$ meV. We note that to simplify the analysis we skip here the spin-orbit coupling between holes in the $xz$ and $yz$ orbitals. Such a simplification is not [a priori]{} justified for a realistic situation in Ca$_2$RuO$_4$ but is rationalised by the intuitive understanding of its spectral functions presented in Ref. , which relies on the Hund’s coupling and does not include the spin-orbit coupling as an essential part. Moreover, a (surprisingly) good agreement between the theoretical results presented below and the experimental results, cf. Fig. \[result\], [a posteriori]{} legitimizes this assumption further. Finally, it will not affect the study of the possible intrinsic differences between the $S=1/2$ and $S=1$ spin polaron models. There are two projections in place in the kinetic Hamiltonian (\[model2\]). First, due to the strong on-site Coulomb repulsion $U$–and since we confine ourselves to the low energy physics valid for energies smaller than the ‘Hubbard’ $U$–we restrict the hole motion to the Hilbert space spanned by the $d^2$ or $d^1$ multiplets on the single ruthenium ions. \[Since the $xy$ orbital is considered to be ‘always’ occupied by two electrons in the studied model [@Mizokawa2001; @Gorelov2010; @Sutter2017], the $xy$ electrons are integrated out and effectively the nominal occupancy of the ruthenium ions is not $d^4$ ($d^3$) but $d^2$ ($d^1$) in the undoped (single-hole) case, respectively.\] As typical to any $t$–$J$-like model [@Chao1977] to formally denote such a constraint we use the tildas above the electron creation and annihilation operators. Second, just as in the case of the ground state (see discussion above), we project the spin $S=0$ states out of the Hilbert space and, formally, Hamiltonian (\[model2\]) contains such projections. We will not, however, keep them explicit in the formulae below. Finally, as we are interested in the photoemission spectrum, we define the following orbitally-resolved hole spectral function, $$\begin{aligned} A_{\alpha}({\bf k}, \omega)\!= \!- \frac{1}{\pi} {\rm Im} \Big\langle 0 \Big\| \tilde{c}^\dag_{{\bf k}, \alpha, \sigma} \frac{1}{\omega - {\mathcal H} + E_0 +i \delta } \tilde{c}_{{\bf k}, \alpha, \sigma} \Big\| 0 \Big\rangle,\end{aligned}$$ where $\| 0 \rangle$ is the ground state of the undoped $t$–$J$ model (\[model1\]-\[model2\]) with energy $E_0$, $\delta$ is the infinitesimally small broadening that is nevertheless finite in the numerical calculations below, and we explicitly keep the orbital index $\alpha \in \{ xz, yz \}$ but suppress the spin index $\sigma$ (the spectral function is spin-independent). In what follows we are also interested in the orbitally-integrated spectral function which is defined in the usual way: $A({\bf k}, \omega)=\sum_{\alpha}A_{\alpha}({\bf k}, \omega)$. From ${\bf t}$-${\bf J}$ to polaron model. {#sec:fromto} ========================================== Stimulated by the successful description of the photoemission spectra of the undoped cuprates [@Wells1995; @LaRosa1997; @Kim1998; @Ramsak1998; @Damascelli2003; @Shen2007; @Manousakis2007; @Wang2015] and to gain a better insight into the physics of the photoemission problem, we perform a mapping of the $S=1$ $t$–$J$ problem onto an $S=1$ spin polaron problem. This is done in two steps: First, we introduce the slave fermions, $$\label{slavefermions} \begin{array}{l} \tilde{c}_{{\bf i},\alpha,\uparrow} \rightarrow h_{{\bf i},\alpha}^{\dag}, \quad \quad \tilde{c}_{{\bf i},\alpha,\downarrow} \rightarrow \hat{A} \: h_{{\bf i},\alpha}^{\dag} \: S_{\bf i}^+,\\ \end{array}$$ where $h_{{\bf i},\alpha}^{\dag}$ is the creation operator for a spinless hole on site $i$ and orbital $\alpha$, $S_{\bf i}^+$ is the spin $S=1$ operator on site ${\bf i}$ and $\hat{A}$ is an operator yet to be determined. It can be shown that in the Hilbert space being considered, that is with the $S=0$ states projected out, the $\hat{A}$ operator is diagonal and an explicit expression for it can be found (see Sec. \[sec:appendix\] for details). Second, we we rotate spins on one of the antiferromagnetic sublattices and express the spin operators through bosonic operators by way of the Holstein-Primakoff transformation. Finally, we use the linear spin wave approximation and the Bogoliubov transformation to diagonalize the resulting spin Hamiltonian–see Sec. \[sec:appendix\] for details. In the end we are left with a diagonal magnon term and a vertex coupling spinless holes to magnons in the following $S=1$ spin polaron Hamiltonian: $$\begin{aligned} \label{finalhamiltonian} H &= H_t + H_J \approx \sum\limits_{\bf q} \: {\Omega}_{\bf q} \: {\beta}_{\bf q}^{\dag} {\beta}_{\bf q} + E_0 \nonumber \\ &+\frac{\sqrt{2} \: t}{\sqrt{N}} \sum\limits_{\textbf{k},\textbf{q}}\Big[\left({\gamma}_{k_{x}}v_{\textbf{q}}+{\gamma}_{k_{x}-q_{x}}u_{\textbf{q}}\right) h_{\textbf{k},xz}^{\dag}h_{\textbf{k}-\textbf{q},xz} {\beta}_{\textbf{q}}\nonumber \\ &+ \left({\gamma}_{k_{y}}v_{\textbf{q}}+{\gamma}_{k_{y}-q_{y}}u_{\textbf{q}}\right) h_{\textbf{k},yz}^{\dag}h_{\textbf{k}-\textbf{q},yz}{\beta}_{\textbf{q}}+h.c. \Big],\end{aligned}$$ where $\gamma_{k_i} = \cos(k_i)$ and $\beta_q$ are the Bogoliubov boson (magnon) annihilation operators. $u_{\bf q}, v_{\bf q}$ are the Bogoliubov coefficients - see Sec. \[sec:appendix\] for details. The above transformations also lead directly to the expression for the spectral function in terms of the spinless hole Green’s function (see Sec. \[sec:appendix\] for details): $$\begin{aligned} A_{\alpha}({\bf k}, \omega)\! =\! - \frac{1}{\pi} {\rm Im} \Big\langle 0 \Big\| {h}_{{\bf k}, \alpha} \frac{1}{\omega - H + E_0 +i \delta } {h}^\dag_{{\bf k}, \alpha} \Big\| 0 \Big\rangle.\end{aligned}$$ Methods and results. {#sec:mandr} ===================== We calculate the hole spectral function $A_{\alpha}({\bf k}, \omega)$ using the self-consistent Born approximation (SCBA), see Ref. [@Martinez1991]. Such approach has been widely-successful in obtaining the cuprate spectral functions [@Martinez1991; @Ramsak1998; @Manousakis2007; @Wang2015; @Bieniasz2018] and amounts to neglecting the so-called crossing diagrams and summing all the other (‘rainbow diagrams’) to infinite order. The resulting self-consistent expressions for the self-energies and the Green’s function are given in Sec. \[sec:appendix\]. These equations are then solved numerically on a finite lattice of $36 \times 36$ ${\bf k}$ points. The resulting orbitally-integrated hole spectral function $A({\bf k}, \omega)$ is calculated for the realistic parameters of the model (see above) and is shown in Fig. \[result\](b). The calculated hole spectral function qualitatively reproduces the incoherent and almost momentum-independent spectrum observed in the high binding energy part of Ca$_2$RuO$_4$ photoemission results found in Ref. and reproduced in Fig. \[result\](a). Although the onset of several horizontal ‘stripes’ in the theoretical spectrum (see below) make the similarities between the theoretical and experimental spectral functions less apparent at first sight \[Fig. \[result\](b)\], a convolution of the theoretical spectral function with the available experimental resolution of ca. $0.5t$ yields a spectrum \[Fig. \[result\](c)\] which surprisingly well resembles the high binding energy part of the observed experimental spectrum \[Fig. \[result\](a)\]: both spectra have an incoherent character, without a clear quasiparticle band emerging, and only very weak dependence of its intensity on the momentum. (A weak dependence on the momentum of the intensities in the high binding energy part of the observed experimental spectrum \[Fig. \[result\](a)\] originates in the $xy$ orbital spectral function, not considered here but explained in detail in Ref. .) What is more, the low- and high-energy edges of both broad spectra are basically momentum-independent. Finally, also the overall energy scale, which is given by the width of the broad spectrum estimated at the half maximum intensity, is of the same order of magnitude in both cases and amounts to about $0.5$ eV. Discussion. {#sec:discussion} =========== What might be the origin of the onset of such an incoherent, almost momentum-independent and, apart from the horizontal ‘stripes’, rather featureless spectrum of Fig. \[result\](b)? Looking first at model (\[model1\]-\[model2\]) we can immediately note what distinguishes it from the ‘standard’ $S=1/2$ $t$–$J$ model, that has been widely used to describe the photoemission spectra of the undoped cuprates [@Schmitt1988; @Martinez1991; @Ramsak1998; @Manousakis2007; @Wang2015] and for which such a broad and flat incoherent band has not been observed. The most apparent are the two anisotropies. The spin anisotropy reflects the distortion of the lattice and leads to the $\gamma$ and $\epsilon$ terms in Eq. (\[model1\]). The perfect hopping anisotropy, on the other hand, which has its origin in the nominal valence of the ruthenium ions and the geometry of the ruthenium-oxide plane, leads to an effectively one-dimensional hole motion, cf. Eq. (\[model2\]). On top of that, a more subtle distinction is related to the larger value of the spin $S=1$ in the studied model. The latter leads to the onset of additional projection operators in the hopping part of the Hamiltonian. ![The hole spectral functions $A({\bf k}, \omega)$ obtained for distinct versions of the relevant $t$–$J$ models and calculated by mapping onto the spin-polaronic model and using the SCBA method (see text): (a) the ‘standard’ spin $S=1/2$ $t$–$J$ model, cf. Ref. ; (b) spin $S=1$ $t$–$J$ model with neither the spin nor the hopping anisotropy, i.e. model (\[model1\]-\[model2\]) with $\varepsilon=\gamma \equiv 0$ and ${\bf e}_{xz}\equiv{\bf e}_{yz} \in \{\hat{x}, \hat{y}\}$; (c) the spin $S=1$ $t$–$J$ model with the hopping anisotropy as suggested for Ca$_2$RuO$_4$ but no spin anisotropy, i.e. model (\[model1\]-\[model2\]) with ${\bf e}_{xz} = \hat{x}$ and ${\bf e}_{yz}=\hat{y}$; and (d) the spin $S=1$ $t$–$J$ model with both anisotropies present as suggested for Ca$_2$RuO$_4$ and equivalent to Fig. \[result\](b), i.e. model (\[model1\]-\[model2\]) with ${\bf e}_{xz} = \hat{x}$, ${\bf e}_{yz}=\hat{y}$, and all model parameters as in Fig. \[result\](b). All spectra normalised as Fig. \[result\]. []{data-label="fourplots"}](fig2.png){width="50.00000%"} We explore the above-listed differences in detail by comparing the spectral function $A({\bf k}, \omega)$ calculated for the distinct versions of the relevant $t$–$J$ models, cf. Fig. \[fourplots\]. Firstly, it is evident that the effects of the spin anisotropy are profound, see Figs. \[fourplots\] (c) and (d). On the one hand, it makes the spectrum less dispersive and in general more featureless; on the other it leads to the formation of a horizontal stripes superimposed onto the otherwise featureless spectrum. Both the former and the latter can be understood, when one considers the fact that the very large anisotropy limit leads, in this case, to the dominant Ising-like interactions between spins. This triggers the hole confinement in a linear string potential and leads to a well-known ladder-like spectrum with the horizontal ‘stripes’ [@Martinez1991; @Dagotto1994; @Bieniasz2018]. ![The one dimensional character of the orbitally-resolved hole spectral function: (a) Constant-energy cut of the spectral function $A_{xz} ({\bf k}, \omega_c)$ for a hole introduced into the $xz$ orbital ($\omega_c = -1.9 $ eV); (b) Constant-energy cut of the spectral function $A_{yz} ({\bf k}, \omega_c)$ for a hole introduced into the $yz$ orbital ($\omega_c = -1.9 $ eV); (c-d) A schematic view of the ruthenium-oxygen plane explaining the dominant one-dimensional character of the electronic hopping processes on the single-particle level that is also inherited by the many-body hopping processes of Eq. (\[model2\]): For the $xz$ ($yz$) orbital, only hopping in the $\hat{x}$ ($\hat{y}$) direction is possible, cf. panel (c) \[(d)\] [@Slater1954; @Harris2004]. The oxygen (ruthenium) orbitals are shown in blue (red).[]{data-label="oned"}](fig3.png){width="50.00000%"} ![A schematic view of the possible nearest neighbor hole hoppings in the $S=1$ and $S=1/2$ antiferromagnet (AF): (Top panel) A hopping process in the $S=1$ antiferromagnet that, according to the here studied $t$–$J$ Hamiltonian (\[model1\]-\[model2\]), leads to the creation of one magnon in the effective $S=1$ spin polaron model (\[finalhamiltonian\]); (Middle panel) An analogous hopping process as above but in the $S=1/2$ antiferromagnet which, according to the ‘standard’ $t$–$J$ Hamiltonian [@Chao1977], leads to the creation of one magnon in the spin polaron model of Ref. ; (Bottom panel) A hopping process in the $S=1$ antiferromagnet that, according to the here studied $t$–$J$ Hamiltonian (\[model1\]-\[model2\]), leads to the creation of three magnons and is [neglected]{} in the $S=1$ spin polaron model (\[finalhamiltonian\]) for it goes beyond the linear spin wave approximation.[]{data-label="hoppingprocesses"}](fig4.png){width="50.00000%"} Secondly, one can see that the one-dimensional hole motion completely changes the character of the spectral function, cf. Fig. \[fourplots\](b) and (c). In order to better understand why this happens, in Fig. \[oned\] we present the constant energy cuts of two spectral functions–one describing a hole in the $xz$ orbital, the other a hole in the $yz$ orbital. We see that the one-dimensional hole motion—a consequence of the geometry of the ruthenium-oxygen plane and the vanishing of the transfer integrals between the oxygen $p$ orbitals and some of the $t_{2g}$ orbitals [@Harris2004]—is reflected in the hole spectral functions. They both show a manifestly one-dimensional dispersion, very much unlike what we see, for instance, in the copper oxides [@Wells1995; @LaRosa1997; @Kim1998; @Damascelli2003; @Shen2007]. We note that, while including a finite spin-orbit coupling for holes in the $xz$ or $yz$ orbitals would naturally lead to the ‘mixing’ between the one-dimensional bands, a good agreement between the theoretical and experimental spectra suggests that such an effect should be small in Ca$_2$RuO$_4$. Finally, with all other parameters equal, the fact that we do not consider here a spin $S=1/2$ (which would be formed by a single hole or electron per site) but a spin $S=1$ antiferromagnet (two holes on each site) does not influence the spectral function qualitatively–thus, the difference between these two cases is purely quantitative, cf. Fig. \[fourplots\](a) and (b). To understand why it is so, let us compare the possible hole hopping processes in the $S=1/2$ and $S=1$ antiferromagnet, which are represented schematically in Fig. \[hoppingprocesses\]. What we can conclude by looking at the process represented on the bottom panel is that all the more complex processes, which have no analog in the single hole per site case, involve more than one magnon. In fact they involve either three or five magnons, which is why we exclude them in the spin wave approximation employed here and why they are absent from Hamiltonian (\[finalhamiltonian\]). Consequently, only the simplest process remains, the one analogous to the only process possible in the spin $S=1/2$ case, cf. the first two panels of Fig. \[hoppingprocesses\]. We stress that such a similarity between the hole moving in the $S=1/2$ and the $S=1$ antiferromagnet would not be achieved in the classical double exchange picture [@Zener1951], for the latter one would not allow for the existence of the $\|1, 0 \rangle$ states on any site. Conclusions. {#sec:conclusions} ============ In this work we showed how a relatively simple spin $S=1$ $t$–$J$ model, that was mapped onto an $S=1$ spin polaron model, can qualitatively reproduce the high-binding energy part of the observed Ca$_2$RuO$_4$ photoemission spectrum. In particular, we were able to explain the observed incoherent and almost momentum-independent photoemission spectrum by linking these peculiar features of the spectrum to two anisotropies present in the employed spin polaron model—the spin anisotropy [@Kunkemoeller2017] and the hopping anisotropy [@Harris2004; @Sutter2017]. Interestingly, the differences between the spectral functions of the ‘standard’ spin polaron model well-known from the cuprates (i.e. spin $S=1/2$) and the model for Ca$_2$RuO$_4$ should not be regarded as being intrinsic to the $S=1$ spin polaron model: They are all solely related to the above-mentioned strong anisotropies present in the model suggested for Ca$_2$RuO$_4$ and [not]{} to the potential differences between the hole moving in the $S=1/2$ and the $S=1$ antiferromagnet. These turn out to be basically irrelevant in the linear spin wave approximation. Such a result can naturally be expected following basic quantum mechanics but would not be achieved in the well-known double exchange picture [@Zener1951], for in that classical approach the hole would not be able to hop at all in the $S=1$ antiferromagnet. Acknowledgments. {#acknowledgments. .unnumbered} ================ We are very grateful to David Sutter and Johan Chang for sharing the experimental data that was presented in Ref. and which allowed us to plot Fig. \[result\](a). We thank Eugenio Paris for insightful discussions. A.K. thanks the IFW Dresden for the kind hospitality. A.K. and K.W. (K.W.) acknowledge(s) support by Narodowe Centrum Nauki (NCN, Poland) under Projects No. 2016/22/E/ST3/00560 (2016/23/B/ST3/00839), respectively. J.v.d.B. acknowledges financial support from the German Research Foundation (Deutsche Forschungsgemeinschaft, DFG) via SFB1143 project A5 and the Würzburg-Dresden Cluster of Excellence ct.qmat. APPENDIX: Derivation of the Polaron model {#sec:appendix .unnumbered} ========================================= Mapping onto a polaronic model: Spin Hamiltonian ($\mathcal{H}_J$) ------------------------------------------------------------------ To diagonalize the spin $S=1$ Hamiltonian discussed in the paper \[cf. Eq. (\[model1\]) of the main text of the paper\] we start by performing two rotations of spins. First, we make a different choice of the spin quantization axis $\hat{z}$ - in this case we pick the axis without an anisotropy term. Second, we perform a $\pi$ rotation of spins around the $\hat{x}$ axis on one of the two sublattices—such transformation maps the anticipated antiferromagnetic ground state onto a ferromagnetic state. The result is the rotated spin Hamiltonian $$\begin{aligned} \label{eq:1} \mathcal{\tilde{H}}_J &= \sum\limits_{\left< {\bf i,j} \right>} J \: \left[ -\: S_{\bf i}^z S_{\bf j}^z + \frac{1}{2} \left( S_{\bf i}^+ S_{\bf j}^+ + S_{\bf i}^- S_j^- \right) \right] \nonumber \\ &+ \gamma \sum\limits_{\bf i}\left(S_{\bf i}^y\right)^2 + \epsilon \sum\limits_{\bf i}\left(S_{\bf i}^x\right)^2.\end{aligned}$$ The next step is to utilize the Holstein-Primakoff transformation and the linear spin wave approximation using the assumption that the ground state is ferromagnetic and dressed with magnons. The thus obtained Hamiltonian is then diagonalized using the successive Fourier and Bogoliubov transformations. The resulting spin Hamiltonian reads $$\begin{aligned} \label{eq:1} {H}_J &= \sum_{\bf q} {\Omega}_{\bf q} \beta^\dag_{\bf q} \beta_{\bf q} \; ,\end{aligned}$$ where the magnon energies $ {\Omega}_{\bf q}$ are given by $${\Omega}_{\bf q} = Y \sqrt{1 - \left( \frac{Z_{\bf q}}{Y} \right)^2},$$ with $$\label{hj solved} \begin{array}{l} Y = 4J+{\epsilon}+{\gamma},\\ Z_{\bf q} = 4J{\gamma}_{\bf q}+{\epsilon}-{\gamma},\\ \end{array}$$ with $$\gamma_{\bf q} = \frac{1}{2} \left( \cos(q_x) + \cos(q_y) \right).$$ The Bogoliubov coefficients $u_{\bf q}$ and $v_{\bf q}$, which describe the connection between the bosons before and after the Bogoliubov transformation and are needed to correctly express the kinetic part of the Hamiltonian in the polaronic language (see next section), are expressed through the magnon energies $ {\Omega}_{\bf q}$ via the standard formulae, cf. Ref. . Mapping onto a polaronic model: Kinetic Hamiltonian ($\mathcal{H}_t$) --------------------------------------------------------------------- ### Dealing with projection operators The implicit projection operators in Eq. (\[model2\]) in the main text have a relatively complex form. The easiest way to deal with them is to construct the projected form of the two single orbital, two-site kinetic Hamiltonians $$\begin{aligned} \label{hamt} (H_t^{xz})_{{\bf i},{\bf i}+{\bf e}_{xz}} &= -t \sum\limits_{\sigma} \tilde{c}_{{\bf i},xz,\sigma}^{\dag}\tilde{c}_{{\bf i}+{\bf e}_{xz},xz,\sigma} + h.c.,\\ \label{hamt2} (H_t^{yz})_{{\bf i},{\bf i}+{\bf e}_{yz}} &= -t \sum\limits_{\sigma} \tilde{c}_{{\bf i},yz,\sigma}^{\dag}\tilde{c}_{{\bf i}+{\bf e}_{yz},yz,\sigma} + h.c.,\end{aligned}$$ step by step, that is by considering every possible hopping process and the matrix element associated with it. We consider a single hole introduced into the half-filled ground state and $H_t$ conserves the number of electrons in the system. Moreover, the ‘no double occupancy’ constraint implies that there can never be 3 electrons on one site in the $xz/yz$ orbitals. As a result, a single hole introduced into the system propagates leaving the number of electrons in the $xz/yz$ orbitals on all other sites unchanged and equal to two. It follows that the only nonzero matrix elements of the two-site Hamiltonians (\[hamt\]-\[hamt2\]) describe processes in which a hole hops between a doubly occupied site and a singly occupied site. Furthermore, these hoppings obey two rules: 1. The hole can hop to the neighbouring site, albeit only to an unoccupied orbital. 2. The hole can hop to the neighbouring site, albeit only if the resulting on-site wavefunction is not a spin singlet. The first rule is simply the ‘no double occupancy’ constraint and the second rule follows from the exclusion of the $S=0$ sector of the Hilbert space discussed in the main text. All of the above means that on each site we have either the spin triplet or one spin $S=1/2$ fermion on the $xz/yz$ orbitals. This in turn implies that for each pair of neighbouring sites ${\bf i,j}$ we can use the following basis $$\label{site basis} \left\{ \Big\| {^{\uparrow}_{\_}} \Big>_{\bf i}, \Big\| {^{\downarrow}_{\_}} \Big>_{\bf i}, \Big\| {^{\_}_{\uparrow}} \Big>_{\bf i}, \Big\| {^{\_}_{\downarrow}} \Big>_{\bf i} \right\} \; \otimes \; \left\{ \Big\| {^{\downarrow}_{\downarrow}} \Big>_{\bf j}, \Big\| {^{\uparrow}_{\uparrow}} \Big>_{\bf j}, \frac{1}{\sqrt{2}} \left( \Big\| {^{\uparrow}_{\downarrow}} \Big> + \Big\| {^{\downarrow}_{\uparrow}} \Big> \right)_{ \bf j} \right\},$$ where the upper and lower positions are the two ($xz/yz$) orbitals, the arrows show spin and the two particle states form the standard triplet. The main task now is to consider the matrix elements of (\[hamt\]-\[hamt2\]) in the basis (\[site basis\]). Because the Hilbert space is 12-dimensional there are 144 different matrix elements. However, it is easy to see that only a small number of them is nonzero. In order to find them one can use a graphical technique ilustrated in Table \[tab:hop\]. The matrix elements listed above and their complex conjugates constitute all nonzero matrix elements. In total there is 32 of them. There are, however, some symmetries that help us write the Hamiltonian in a simpler form. First, $(M_1,M_2,M_5,M_6,M_9,M_{10},M_{13},M_{14})$ and conjugates come from $(H_t^{xz})_{{\bf i},{\bf i}+{\bf e}_{xz}}$, the rest comes from $(H_t^{yz})_{{\bf i},{\bf i}+{\bf e}_{yz}}$. We only need to consider one of these Hamiltonians as the matrix elements of other one can be obtained in an analogous way. From now on we will only consider $(H_t^{xz})_{{\bf i},{\bf i}+{\bf e}_{xz}}$. Second, let us look at $M_4$ and $M_{11}^$ or $M_{11}$ and $M_{4}^$, where a star denotes complex conjugation. They represent exactly the same process but happening in the opposite direction on the lattice. $M_4$ and $M_{11}$ on the other hand represent the inverse processes happening in opposite directions on the lattice. This means we need only calculate one of these matrix elements. The same is true for the pair $(M_8,M_{16})$ and their conjugates. This leaves us with $(M_3,M_4,M_7,M_8,M_{12},M_{15})$. Third, $(M_3,M_7)$ are the same but have all spins flipped, which is a symmetry of the Hamiltonian. The same is true for $(M_4,M_8)$ and $(M_{12},M_{15})$. Altogether, this leaves us with the classification of the nonzero matrix elements shown in Table \[tab:second\]. In order to obtain the second quantised form of (\[hamt\]-\[hamt2\]) we need to calculate all matrix elements after which we can construct the projected two-site Hamiltonian using $$\label{conc ham} (H_t^{xz})_{{\bf i},{\bf i}+{\bf e}_{xz}} = \sum\limits_{k,l} (H_t^{xz})_{{\bf i},{\bf i}+{\bf e}_{xz}}^{k,l} \left\| k \right> \left< l \right\|,$$ where the vectors $\left\| k \right>, \left\| l \right>$ are written in the second quantised form. $(H_t^{xz})_{{\bf i},{\bf i}+{\bf e}_{xz}}^{k,l} \equiv M_j$ are the matrix elements that have been discussed above and need to be explicitly calculated, see below. ### Calculation of the matrix elements The matrix elements $M_j$ can be calculated in a straightforward way. As an example we calculate $M_3$: $$\begin{aligned} M_{3} & =\bigg(\left< 0 \right\| \tilde{c}_{{\bf i},yz,\uparrow}\tilde{c}_{{\bf j},xz,\uparrow}\tilde{c}_{{\bf j},yz,\uparrow} \bigg) \bigg( -t \: \tilde{c}_{{\bf j},xz,\uparrow}^{\dag}\tilde{c}_{{\bf i},xz,\uparrow} \bigg) \nonumber \\ & \times \bigg( \tilde{c}_{{\bf j},yz,\uparrow}^{\dag}\tilde{c}_{{\bf i},yz,\uparrow}^{\dag}\tilde{c}_{{\bf i},xz,\uparrow}^{\dag}\left\| 0 \right>\bigg)\nonumber \\ & =t \: \left< 0 \| 0 \right>.\end{aligned}$$ $M_4$ and $M_{15}$ are calculated in a similar manner. The result is shown in Table \[tab:result\]. Once all the matrix elements are calculated one can easily write down the projected form of Eq. (\[model2\]) in the main text in the second quantized form. ### Polaronic mapping In order to map our model onto a polaronic one, we need to introduce slave fermions (cf. Ref ) using a general mapping $$\label{slavefermions} \begin{array}{l} \tilde{c}_{{\bf i},\alpha,\uparrow} \rightarrow h_{{\bf i},\alpha}^{\dag}, \quad \quad \tilde{c}_{{\bf i},\alpha,\downarrow} \rightarrow \hat{A} \: h_{{\bf i},\alpha}^{\dag} \: S_{\bf i}^+,\\ \end{array}$$ where $\hat{A}$ is an operator to be determined. The spinless hole operators $h_{{\bf i},\alpha}$ obey the Pauli exclusion principle and the standard anticommutation relations. The spin $S=1$ operators obey the standard commutation relations. Finally, the spinles hole operators commute with the spin operators, which introduces an extra term in the Hamiltonian (see below). ### Finding ${\bf \hat{A}}$ After transformation (\[slavefermions\]) the on-site Fock basis consists of the spinless holes with two orbital flavors $xz, yz$ and three eigenvalues of the projection of the spin $S=1$ onto the $\hat{z}$ axis ($S_z$). Thus, we label these states by the number of spinless holes on each orbital $n_{xz}, n_{yz} \in \{ 0,1\}$ and the $S_z \in \{-1,0,1\}$ spin quantum number and write the basis states as $\left\{ \left\| n_{xz}, n_{yz}, S_z \right> \right\}$. To see how the transformation works let us look at the state $\left\| {^-_{\downarrow}} \right>$ ($\left\| 0 \right> \: \equiv \: \left\| 1,1,1 \right>$ defines the vacuum): $$\begin{aligned} \label{example state} \Big\| {^-_{\downarrow}} \Big> &= \sqrt{2} \tilde{c}_{xz , \uparrow} \left( \frac{1}{\sqrt{2}}S^{-} \right) \tilde{c}_{yz , \uparrow}^{\dag} \tilde{c}_{xz , \uparrow}^{\dag} \left\| 0 \right> \nonumber\\ &= \sqrt{2} h_{xz}^{\dag} \left( \frac{1}{\sqrt{2}}S^{-} \right) h_{yz}h_{xz} \left\| 1,1,1 \right> = \sqrt{2} \left\| 1,0,0 \right>. \end{aligned}$$ Thus, the state $\Big\| {^-_{\downarrow}} \Big>$ maps to the state $\sqrt{2} \left\| 1,0,0 \right>$—a state of one hole and one magnon. Similarly, one can determine the other states $$\label{basis map} \begin{array}{ll} \Big\| 0 \Big> \equiv \left\| 1,1,1 \right>, \; & \Big\| {^{\uparrow}_-} \Big> \equiv \left\| 0,1,1 \right>,\\ \Big\| {^{\uparrow}_{\uparrow}} \Big> \equiv \left\| 0,0,1 \right>, \; & \Big\| {^-_{\uparrow}} \Big> \equiv \left\| 1,0,1 \right>,\\ \Big\| {^{\uparrow}_{\downarrow}} \Big> \equiv \left\| 0,0,0 \right>, \; & \Big\| {^{\downarrow}_-} \Big> \equiv \sqrt{2} \left\| 0,1,0 \right>,\\ \Big\| {^{\downarrow}_{\downarrow}} \Big> \equiv \left\| 0,0,-1 \right>, \; & \Big\| {^-_{\downarrow}} \Big> \equiv \sqrt{2} \left\| 1,0,0 \right>.\\ \end{array}$$ We stress that in the above notation the first two quntum numbers are the number of holes on each orbital. \[For example, the state $\left\| 1, 1, 1 \right>$ is the vacuum (no electrons) and the state $\left\| 0, 0, 0 \right>$ is the $S_z = 0$ two electron state.\]. The operator $\hat{A}$ is necessary to normalize the states in the new basis. In (\[basis map\]) we see that two states are not normalized and acquire a factor of $\sqrt{2}$, which is a consequence of the projection onto the $S_z=0$ triplet state. It is easy to check that consequently $\hat{A} = 1$ for $\{ \left\|1,0,0\right>, \left\|0,1,0\right> \}$ and $\hat{A} = \frac{1}{\sqrt{2}}$ otherwise. ### Restricting the Hilbert space Looking at (\[basis map\]) again, we observe that there are four states that do not map to any states in the old basis, namely $$\left\{ \left\| 1,0,-1 \right> , \left\| 0,1,-1 \right> , \left\| 1,1,0 \right> , \left\| 1,1,-1 \right> \right\}.$$ Evidently, these need to be projected out. One could achieve this using projection operators, but it would complicate the formula for the Hamiltonian. Another approach, presented in Ref. for the $S=1/2$ case, is to include an extra term in the Hamiltonian with a very large coupling constant $\zeta > 0$, in the spirit of the Lagrange multipliers. In our case this term takes the form $$\begin{aligned} \label{constraint} \begin{split} H_{\zeta} &= \zeta \sum\limits_{\bf i} \Big[ \left( h_{{\bf i} , xz}^{\dag}h_{{\bf i} , xz} h_{{\bf i} , yz}^{\dag}h_{{\bf i} , yz} \left( S_{\bf i}^z \right)^2 \right) +\\ &+ \left( h_{{\bf i} , xz}^{\dag}h_{{\bf i} , xz} + h_{{\bf i} , yz}^{\dag}h_{{\bf i} , yz} \right) \left( S_{\bf i}^z - 1 \right) S_{\bf i}^z \Big].\\ \end{split}\end{aligned}$$ Following the authors of Ref. we will neglect this part of the Hamiltonian. It is clear that this is not without consequence. For simpler models it was shown [@Bieniasz2018] that including such constraints in the diagrammatic expansion of the Dyson equation leads to quantitative differences. We believe that the same situation happens for the $S=1$ case studied here. ### The linear spin wave (LSW) approximation To arrive at the formula (5) in the main text we need to find the expressions for the operators $\big\| k \big> \big< l \big\|$ appearing in Eq. (\[conc ham\]). We look for them in the LSW approximation. After introducing magnons via the Holstein-Primakoff transformation, the spin quantum number $S_z$ maps onto the number of magnons quantum number $n_{mag}$: $$S_z= 1,0,-1 \rightarrow n_{mag}= 0,1,2 \ ,$$ respectively, while the fermionic quantum numbers $\{ n_{xz}, n_{yz} \}$ remain the same. In this basis, let us examine the projection operator ($P_3$) associated with the matrix element $M_3$ that was discussed above (the other cases are analogous, see below). After the sublattice rotation we obtain $$\begin{aligned} P_{3} &= \Big\| {^{-}_{\uparrow}} \Big>_{{\bf i}} \Big\| {^{\downarrow}_{\downarrow}} \Big>_{{\bf j}} \Big< {^{\uparrow}_{\uparrow}} \Big\|_{{\bf i}} \Big< {^{-}_{\downarrow}} \Big\|_{{\bf j}} = \nonumber \\ &= \sqrt{2} \: \left\| 1,0,0 \right>_{\bf i} \left\| 0,0,2 \right>_{{\bf j}} \left< 0,0,0 \right\|_{\bf i} \left< 1,0,1 \right\|_{{\bf j}} = \nonumber \\ &= \sqrt{2} \: \left( h_{{\bf j},yz} h_{{\bf j},xz} h_{{\bf i},yz} a_{{\bf j}}^{\dag}a_{{\bf j}}^{\dag} \left\| 1,1,0 \right>_{\bf i} \left\| 1,1,0 \right>_{{\bf j}} \right) \nonumber \\ &\otimes \left( \left< 1,1,0 \right\|_{{\bf i}} \left< 1,1,0 \right\|_{{\bf j}} a_{{\bf j}} h_{{\bf j},yz}^{\dag} h_{{\bf i},xz}^{\dag} h_{{\bf i},yz}^{\dag} \right). \end{aligned}$$ First, we notice that the projection onto the double vacuum state, which represents two empty sites, is obsolete. Indeed, if a state survives the action of the spinless fermion creation operators on the right it survives it as one of two states: 1. A state with four spinless holes, two on each site, in which case the projection is obsolete as this is a unique property of the vacuum, 2. A state with three spinless holes, two on the $i$-th site and one on the $i+1$-st site. In this case the annihilation operators on the left annihilate it, because two of them act on the $i+1$-st site. It is easy to see that the same is true for any of the 16 operators multiplying the matrix elements in Table \[tab:hop\] and their Hermitean conjugates. Using this we can write $P_3$ as $$\begin{aligned} P_{3} &= \sqrt{2} \: h_{{\bf j},yz} h_{{\bf j},xz} h_{{\bf i},yz} h_{{\bf j},yz}^{\dag} h_{{\bf i},xz}^{\dag} h_{{\bf i},yz}^{\dag} a_{{\bf j}}^{\dag}a_{{\bf j}}^{\dag} a_{{\bf j}} \nonumber \\ & \approx \sqrt{2} \: h_{{\bf i},xz}^{\dag} h_{{\bf j},xz} a_{{\bf j}}^{\dag}a_{{\bf j}}^{\dag} a_{{\bf j}},\end{aligned}$$ where we have neglected the normal ordered terms with three or more spinless hole operators which go beyond our diagrammatic expansion (see section D). We see that $P_3$ is of order three in the bosonic operators. Performing similar calculations for the other 15 operators one can show that they can be divided into three groups: 1. of order one in bosonic operators, 2. of order three in bosonic operators, 3. of order five in bosonic operators. In the LSW approximation we only consider the first group of terms. Consequently, only four amongst the 16 operators are non-negligible. These are $ \{ P_2 , P_4, P_{10}, P_{16} \} $. Together with their respective matrix elements the four operators and their Hermitean conjugates give the projected kinetic Hamiltonian in the LSW approximation, see last two lines of Eq. (\[finalhamiltonian\]) in the main text. Mapping onto a polaronic model: Spectral functions -------------------------------------------------- As discussed in the main text of the paper we are interested in calculating the following spectra function $$\begin{aligned} &{A}_{\alpha}({\bf k},\omega) = -\frac{1}{\pi} {\rm Im}\left\{{G}_{\alpha}({\bf k},\omega) \right\} = \nonumber \\ &= -\frac{1}{\pi} {\rm Im} \left\langle 0 \right\| \tilde{c}^{\dag}_{{\bf k},\alpha,\sigma} \frac{1}{\omega - \mathcal{H} + E_0 + i \delta} \tilde{c}_{{\bf k},\alpha\sigma} \left\| 0 \right\rangle,\end{aligned}$$ where $\tilde{c}_{{\bf k},\alpha,\sigma} = c_{{\bf k},\alpha,\sigma}(1-c^{\dag}_{{\bf k},\alpha,{\bar \sigma}}c_{{\bf k},\alpha,{\bar \sigma}})$ are the restricted hole annihilation operators. It is therefore not a one particle Green’s function. The relation between the above-defined hole spectral function and the spinless hole spectral function is nontrivial, cf. Appendix of Ref. . The latter one, that is natural to the polaronic language, is calculated from the single-particle spinless hole Green’s function and reads $$\begin{aligned} \label{spectral ok} &A_{\alpha}({\bf k},\omega) = -\frac{1}{\pi} {\rm Im}\left\{ G_{\alpha}({\bf k},\omega) \right\} = \nonumber \\ &=-\frac{1}{\pi} {\rm Im } \left\langle 0 \right\| h_{{\bf k},\alpha} \frac{1}{\omega - H +E_0 + i \delta} h^{\dag}_{{\bf k},\alpha} \left\| 0 \right\rangle.\end{aligned}$$ Fortunately, it was shown that for the $S=1/2$ $t$-$J$ model the spinless hole spectral function and the hole spectral function almost coincide [@Wang2015]. We assume that the same also holds also for the $S=1$ $t$-$J$ model investigated here. The self-consistent Born approximation to the Dyson equation {#sec:scba} ------------------------------------------------------------ To obtain the Green’s function $G_{\alpha}({\bf k},\omega)$ of Eq. (\[spectral ok\]), and thus calculate the spectral function $A_{\alpha}({\bf k},\omega)$, we use the Dyson equation that reads $$G_{\alpha}({\bf k},\omega) = G^{0}_{\alpha}({\bf k},\omega) + G^{0}_{\alpha}({\bf k},\omega) \Sigma_{\alpha}({\bf k},\omega) G_{\alpha}({\bf k},\omega),$$ where $\alpha$ is an orbital index. The self energy $\Sigma_{\alpha}({\bf k},\omega)$ is defined as the sum of all non-reducible diagrams starting and ending with the same vertex with an external line representing a spinless hole with momentum ${\bf k}$ and orbital index $\alpha$. We calculate the self energy $\Sigma_{\alpha}({\bf k},\omega)$ approximately, using the self-consistent Born approximation (SCBA): $$\begin{aligned} \label{scba diag} \begin{split} &\Sigma_{\alpha}({\bf k},\omega) \approx \\ &= \int\limits_{-\infty}^{\infty} d \omega' \sum\limits_{{\bf q}} \; D^{0}(\omega') G_{\alpha}({\bf k} - {\bf q}, \omega - \omega') V_{\alpha} ({\bf k}, {\bf q}) V_{\alpha} ({\bf k}, {\bf q})^, \end{split}\end{aligned}$$ where the vertex is defined as $$\begin{aligned} \label{vertex} \begin{split} V_{\alpha} \left( {\bf k}, {\bf q} \right) &= \frac{\sqrt{2} \: t}{\sqrt{N}} \ \left({\gamma}_{{\bf k} \cdot {\bf e}_{\alpha}} v_{\textbf{q}}+{\gamma}_{({\bf k-q}) \cdot {\bf e}_{\alpha}} u_{\textbf{q}} \right), \\ \end{split}\end{aligned}$$ and the magnon Green’s function is $$\label{magnongreen} D^{0}(\omega) = \delta(\omega - \Omega_{\bf q}).$$ Using Eqs. 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Susceptibility of TNF-alpha-deficient mice to Trypanosoma congolense is not due to a defective antibody response. C57BL/6 mice deficient in one or two copies of the gene for tumor necrosis factor alpha (TNF-alpha) were more susceptible to Trypanosoma congolense infection than their resistant, wild-type counterparts. The number of TNF-alpha genes was correlated with the capacity to control parasitaemia and with survival time. Absence of TNF-alpha resulted in a diminished capacity to form germinal centres in lymph nodes and spleen. Since germinal centres are involved in antibody production and affinity maturation, the susceptibility of the TNF-alpha-deficient mice could have been due to this secondary defect. Despite the lack of the germinal centres, the antibody responses to internal and exposed trypanosome antigens and to non-trypanosome antigens were not significantly different. Also the relative avidities measured in infected sera did not significantly differ between the two mouse strains. These data suggest that the role of TNF-alpha in control of T. congolense was not due to its role in the development of an antibody response.	{ "pile_set_name": "PubMed Abstracts" }
Honorable Mention #1 The Starship Creator series Honorable Mention #2 Starfleet Command 2: Community Edition Star Trek has been a staple of video games almost from the beginning of the medium. So it's no surprise that there's a huge list of Star Trek video games out there, with output peaking in the 1990's, a time when producing games was a whole lot cheaper because everything was a lot less sophisticated. But as Trek game production slowed to a trickle due to legal disputes and bad decisions, many Trek gamers have been looking to the past to get their fix. One problem with playing 20+ year old games is the fact that a lot of them are subpar on the technical front and often technologically incompatible with newer systems (including PCs). And to make things worse, the oldest games aren't all that friendly to those who don't have the manuals or can't handle the extreme levels of micromanagement that some of these games involve. But with HD remakes being all the rage these days, now seems like a good time to revamp games that many Trekkers might not be familiar with. So here are 7 Star Trek games that deserve a chance to see the light of day in HD.More of a simulation than a game, the Starship creator series gave Trek fans an opportunity to design their own custom versions of iconic starships, customize their internals, crew them with numerous Trek characters or custom characters of their own making, and send them on missions to test the ships' abilities. Sadly, what sounds awesome on paper didn't make for an exciting piece of software. A limited amount of ships, almost all Federation except for the Klingon Bird of Prey included in Warp II, an economy driven building system that require grinding through missions for money, and a terrible mission system that boiled down to watching dots and icons moving around sucked all the life out of the game. In an ironic twist of fate, Star Trek Online's ship customization replicates the ship design elements of Starship Creator with a larger selection of ships and options (including color customization). The only real difference is that there's none of the in-depth internal customization that Starship Creator had. Unfortunately, the only way to use this is to actually play STO, which probably isn't ideal for anyone who hates MMOs and/or free-to-play games.The Starfleet Command (SFC) series of starship combat games is heavily based on the Starfleet Battles tabletop games (aka Star Trek: Every Ship Has Planet Destroying Firepower). With two Original Series movie era games and Next Generation era one that received, SFC was one of the bigger subfranchises in Trek gaming before Activision sued Paramount and killed Trek gaming for a few years. But in one of the most astounding and incomprehensible turns in video game history, a non-profit organization known as the Dynaverse Gaming Association obtained the rights to the entire series, including the rare SFC3 (which isn't sold on their site). One of their major projects, which recently reached completion after eight years of development, was Starfleet Command 2: Community Edition. While not a legitimate HD remaster, it did revamp the technical underpinnings of the game, making it fully compatible with modern Windows operating systems. While the game still looks oddly outdated and is horrifically complex to control for newcomers, it's a great gift to an old, loyal fanbase that has managed to last through the years.	{ "pile_set_name": "OpenWebText2" }
Resolve references to extern crate root in paths without extern crate item for 2018 edition Support multiple definitions in lazy_static macro call (by @msmorgan ) Allow modifying loop variable name generated by iter postfix template (by @Voronchikhin ) Add examples for all postfix templates Use offline mode for cargo sync if the corresponding option is enabled Improve content roots detection. Now src , examples , tests and benches folders of each package are automatically marked as source roots, and target folders are excluded from source roots Fix name resolution of stdlib macros for nightly stdlib Make Move Statement Up/Down actions work correctly Process global imports in use group while name resolution in proper way Partially resolve links which based on re-exported paths in stdlib documentation	{ "pile_set_name": "OpenWebText2" }
Sharp considers chairman's retirement, to scrap posts: Kyodo Published May 05, 2013 Reuters Copyright Reuters 2013 TOKYO – Japan's Sharp Corp is considering having its chairman, Mikio Katayama, retire and also scrapping advisory posts as part of efforts to speed up a business revival under its president, Takashi Okuda, Kyodo news agency reported on Sunday. Sharp, Japan's leading maker of liquid crystal displays, is expected to reveal a medium-term business management plan on May 14. It wants a new management structure for a business rebuilding with authority concentrated with Okuda, the news agency said. The company's main creditor banks, Mizuho Corporate Bank and the Bank of Tokyo-Mitsubishi UFJ, have been seeking Katayama's retirement because his presence caused uncertainty in the decision-making process and his retirement was considered unavoidable, Kyodo said. Company spokesmen were not available for comment. The Yomiuri newspaper said Katayama has already notified creditors of his intention to step down. Kyodo also said a company adviser, Katsuhiko Machida, and a special adviser, Haruo Tsuji, were expected to retire and the company would probably abolish those posts. This month, two sources with knowledge of Sharp's earnings told Reuters that it posted a worse than forecast 500 billion yen ($5.1 billion) net loss in the year that ended on March 31 as panel plants asset write offs crimped its bottom line.	{ "pile_set_name": "Pile-CC" }
Q: What Bible translations are accepted by the Southern Baptist Convention? Is there is a list of which translations of the Bible are accepted by the Southern Baptist Convention? A: The Southern Baptist Convention, while the highest authority within the Southern Baptist church, is not technically an authority amongst Baptists. It functions as a voluntary association with which member churches may choose to associate, but cannot dictate terms to anyone. While it does approve changes to the "Baptist Faith and Message," these are to be taken as guidelines not at odds with the local autonomy of the church. Within the Baptist Faith and Message (the closest thing Baptists have to a creed), it simply says: The Holy Bible was written by men divinely inspired and is God's revelation of Himself to man. It is a perfect treasure of divine instruction. It has God for its author, salvation for its end, and truth, without any mixture of error, for its matter. Therefore, all Scripture is totally true and trustworthy. It reveals the principles by which God judges us, and therefore is, and will remain to the end of the world, the true center of Christian union, and the supreme standard by which all human conduct, creeds, and religious opinions should be tried. All Scripture is a testimony to Christ, who is Himself the focus of divine revelation. The BFM itself is silent on which versions are "approved." That said, I suspect the question wants to know what translations are preferred. Here, any major translation would suffice, I propose the following list to help you figure out which ones are most likely: Conservative to Evangelical: English Standard Version (ESV), NIV, HCSB (if you went to Dallas Theological Seminary) Moderate to Scholarly: NRSV, RSV Moderate to Gender-inclusively liberal: TNIV Super-traditional: King James Version. Maybe New King James, if they're feeling special. Conservative but Scholarly: The Amplified Bible. When the Preacher wants to make a point: NLT, "The Message" Perhaps more useful would be the ones Baptists would be very unlikely to use: New Jerusalem Bible, Duoay-Rheims: perceived as too Catholic New World Translation: restricted to the Jehovah's Witness Makes most conservatives barf: The Living Bible, Readers Digest Condensed, Good News Translation.	{ "pile_set_name": "StackExchange" }
> \brief \b DGGQRF * =========== DOCUMENTATION =========== * * Online html documentation available at * http://www.netlib.org/lapack/explore-html/ * > \htmlonly > Download DGGQRF + dependencies > <a href="http://www.netlib.org/cgi-bin/netlibfiles.tgz?format=tgz&filename=/lapack/lapack_routine/dggqrf.f"> > [TGZ]</a> > <a href="http://www.netlib.org/cgi-bin/netlibfiles.zip?format=zip&filename=/lapack/lapack_routine/dggqrf.f"> > [ZIP]</a> > <a href="http://www.netlib.org/cgi-bin/netlibfiles.txt?format=txt&filename=/lapack/lapack_routine/dggqrf.f"> > [TXT]</a> > \endhtmlonly * Definition: * =========== * * SUBROUTINE DGGQRF( N, M, P, A, LDA, TAUA, B, LDB, TAUB, WORK, * LWORK, INFO ) * * .. Scalar Arguments .. * INTEGER INFO, LDA, LDB, LWORK, M, N, P * .. * .. Array Arguments .. * DOUBLE PRECISION A( LDA, * ), B( LDB, * ), TAUA( * ), TAUB( * ), * $ WORK( * ) * .. * * > \par Purpose: ============= > > \verbatim > > DGGQRF computes a generalized QR factorization of an N-by-M matrix A > and an N-by-P matrix B: > > A = QR, B = QTZ, > > where Q is an N-by-N orthogonal matrix, Z is a P-by-P orthogonal > matrix, and R and T assume one of the forms: > > if N >= M, R = ( R11 ) M , or if N < M, R = ( R11 R12 ) N, > ( 0 ) N-M N M-N > M > > where R11 is upper triangular, and > > if N <= P, T = ( 0 T12 ) N, or if N > P, T = ( T11 ) N-P, > P-N N ( T21 ) P > P > > where T12 or T21 is upper triangular. > > In particular, if B is square and nonsingular, the GQR factorization > of A and B implicitly gives the QR factorization of inv(B)A: > > inv(B)A = Z*T(inv(T)R) > > where inv(B) denotes the inverse of the matrix B, and ZT denotes the > transpose of the matrix Z. > \endverbatim * Arguments: * ========== * > \param[in] N > \verbatim > N is INTEGER > The number of rows of the matrices A and B. N >= 0. > \endverbatim > > \param[in] M > \verbatim > M is INTEGER > The number of columns of the matrix A. M >= 0. > \endverbatim > > \param[in] P > \verbatim > P is INTEGER > The number of columns of the matrix B. P >= 0. > \endverbatim > > \param[in,out] A > \verbatim > A is DOUBLE PRECISION array, dimension (LDA,M) > On entry, the N-by-M matrix A. > On exit, the elements on and above the diagonal of the array > contain the min(N,M)-by-M upper trapezoidal matrix R (R is > upper triangular if N >= M); the elements below the diagonal, > with the array TAUA, represent the orthogonal matrix Q as a > product of min(N,M) elementary reflectors (see Further > Details). > \endverbatim > > \param[in] LDA > \verbatim > LDA is INTEGER > The leading dimension of the array A. LDA >= max(1,N). > \endverbatim > > \param[out] TAUA > \verbatim > TAUA is DOUBLE PRECISION array, dimension (min(N,M)) > The scalar factors of the elementary reflectors which > represent the orthogonal matrix Q (see Further Details). > \endverbatim > > \param[in,out] B > \verbatim > B is DOUBLE PRECISION array, dimension (LDB,P) > On entry, the N-by-P matrix B. > On exit, if N <= P, the upper triangle of the subarray > B(1:N,P-N+1:P) contains the N-by-N upper triangular matrix T; > if N > P, the elements on and above the (N-P)-th subdiagonal > contain the N-by-P upper trapezoidal matrix T; the remaining > elements, with the array TAUB, represent the orthogonal > matrix Z as a product of elementary reflectors (see Further > Details). > \endverbatim > > \param[in] LDB > \verbatim > LDB is INTEGER > The leading dimension of the array B. LDB >= max(1,N). > \endverbatim > > \param[out] TAUB > \verbatim > TAUB is DOUBLE PRECISION array, dimension (min(N,P)) > The scalar factors of the elementary reflectors which > represent the orthogonal matrix Z (see Further Details). > \endverbatim > > \param[out] WORK > \verbatim > WORK is DOUBLE PRECISION array, dimension (MAX(1,LWORK)) > On exit, if INFO = 0, WORK(1) returns the optimal LWORK. > \endverbatim > > \param[in] LWORK > \verbatim > LWORK is INTEGER > The dimension of the array WORK. LWORK >= max(1,N,M,P). > For optimum performance LWORK >= max(N,M,P)max(NB1,NB2,NB3), > where NB1 is the optimal blocksize for the QR factorization > of an N-by-M matrix, NB2 is the optimal blocksize for the > RQ factorization of an N-by-P matrix, and NB3 is the optimal > blocksize for a call of DORMQR. > > If LWORK = -1, then a workspace query is assumed; the routine > only calculates the optimal size of the WORK array, returns > this value as the first entry of the WORK array, and no error > message related to LWORK is issued by XERBLA. > \endverbatim > > \param[out] INFO > \verbatim > INFO is INTEGER > = 0: successful exit > < 0: if INFO = -i, the i-th argument had an illegal value. > \endverbatim * * Authors: * ======== * > \author Univ. of Tennessee > \author Univ. of California Berkeley > \author Univ. of Colorado Denver > \author NAG Ltd. * > \date December 2016 > \ingroup doubleOTHERcomputational > \par Further Details: ===================== > > \verbatim > > The matrix Q is represented as a product of elementary reflectors > > Q = H(1) H(2) . . . H(k), where k = min(n,m). > > Each H(i) has the form > > H(i) = I - taua * v * v*T > > where taua is a real scalar, and v is a real vector with > v(1:i-1) = 0 and v(i) = 1; v(i+1:n) is stored on exit in A(i+1:n,i), > and taua in TAUA(i). > To form Q explicitly, use LAPACK subroutine DORGQR. > To use Q to update another matrix, use LAPACK subroutine DORMQR. > > The matrix Z is represented as a product of elementary reflectors > > Z = H(1) H(2) . . . H(k), where k = min(n,p). > > Each H(i) has the form > > H(i) = I - taub v * v*T > > where taub is a real scalar, and v is a real vector with > v(p-k+i+1:p) = 0 and v(p-k+i) = 1; v(1:p-k+i-1) is stored on exit in > B(n-k+i,1:p-k+i-1), and taub in TAUB(i). > To form Z explicitly, use LAPACK subroutine DORGRQ. > To use Z to update another matrix, use LAPACK subroutine DORMRQ. > \endverbatim > ===================================================================== SUBROUTINE DGGQRF( N, M, P, A, LDA, TAUA, B, LDB, TAUB, WORK, $ LWORK, INFO ) * * -- LAPACK computational routine (version 3.7.0) -- * -- LAPACK is a software package provided by Univ. of Tennessee, -- * -- Univ. of California Berkeley, Univ. of Colorado Denver and NAG Ltd..-- * December 2016 * * .. Scalar Arguments .. INTEGER INFO, LDA, LDB, LWORK, M, N, P * .. * .. Array Arguments .. DOUBLE PRECISION A( LDA, * ), B( LDB, * ), TAUA( * ), TAUB( * ), $ WORK( * ) * .. * * ===================================================================== * * .. Local Scalars .. LOGICAL LQUERY INTEGER LOPT, LWKOPT, NB, NB1, NB2, NB3 * .. * .. External Subroutines .. EXTERNAL DGEQRF, DGERQF, DORMQR, XERBLA * .. * .. External Functions .. INTEGER ILAENV EXTERNAL ILAENV * .. * .. Intrinsic Functions .. INTRINSIC INT, MAX, MIN * .. * .. Executable Statements .. * * Test the input parameters * INFO = 0 NB1 = ILAENV( 1, 'DGEQRF', ' ', N, M, -1, -1 ) NB2 = ILAENV( 1, 'DGERQF', ' ', N, P, -1, -1 ) NB3 = ILAENV( 1, 'DORMQR', ' ', N, M, P, -1 ) NB = MAX( NB1, NB2, NB3 ) LWKOPT = MAX( N, M, P )NB WORK( 1 ) = LWKOPT LQUERY = ( LWORK.EQ.-1 ) IF( N.LT.0 ) THEN INFO = -1 ELSE IF( M.LT.0 ) THEN INFO = -2 ELSE IF( P.LT.0 ) THEN INFO = -3 ELSE IF( LDA.LT.MAX( 1, N ) ) THEN INFO = -5 ELSE IF( LDB.LT.MAX( 1, N ) ) THEN INFO = -8 ELSE IF( LWORK.LT.MAX( 1, N, M, P ) .AND. .NOT.LQUERY ) THEN INFO = -11 END IF IF( INFO.NE.0 ) THEN CALL XERBLA( 'DGGQRF', -INFO ) RETURN ELSE IF( LQUERY ) THEN RETURN END IF * QR factorization of N-by-M matrix A: A = QR CALL DGEQRF( N, M, A, LDA, TAUA, WORK, LWORK, INFO ) LOPT = WORK( 1 ) * * Update B := Q*TB. * CALL DORMQR( 'Left', 'Transpose', N, P, MIN( N, M ), A, LDA, TAUA, $ B, LDB, WORK, LWORK, INFO ) LOPT = MAX( LOPT, INT( WORK( 1 ) ) ) * * RQ factorization of N-by-P matrix B: B = TZ. CALL DGERQF( N, P, B, LDB, TAUB, WORK, LWORK, INFO ) WORK( 1 ) = MAX( LOPT, INT( WORK( 1 ) ) ) * RETURN * * End of DGGQRF * END	{ "pile_set_name": "Github" }
A₁ adenosine receptor modulation of chemically and electrically evoked lumbar locomotor network activity in isolated newborn rat spinal cords. It is not well-studied how the ubiquitous neuromodulator adenosine (ADO) affects mammalian locomotor network activities. We analyzed this here with focus on roles of 8-cyclopentyl-1,3-dipropylxanthine (DPCPX)-sensitive A(1)-type ADO receptors. For this, we recorded field potentials from ventral lumbar nerve roots and electrically stimulated dorsal roots in isolated newborn rat spinal cords. At ≥ 25μM, bath-applied ADO slowed synchronous bursting upon blockade of anion-channel-mediated synaptic inhibition by bicuculline (20 μM) plus strychnine (1 μM) and this depression was countered by DPCPX (1 μM) as tested at 100 μM ADO. ADO abolished this disinhibited rhythm at ≥ 500 μM. Contrary, the single electrical pulse-evoked dorsal root reflex, which was enhanced in bicuculline/strychnine-containing solution, persisted at all ADO doses (5 μM-2 mM). In control solution, ≥ 500 μM ADO depressed this reflex and pulse train-evoked bouts of alternating fictive locomotion; this inhibition was reversed by 1 μM DPCPX. ADO (5 μM-2 mM) did not depress, but stabilize alternating fictive locomotion evoked by serotonin (10 μM) plus N-methyl-d-aspartate (4-5 μM). Addition of DPCPX (1μM) to control solution did not change either the dorsal root reflex or rhythmic activities indicating lack of endogenous A(1) receptor activity. Our findings show A(1) receptor involvement in ADO depression of the dorsal root reflex, electrically evoked fictive locomotion and spontaneous disinhibited lumbar motor bursting. Contrary, chemically evoked fictive locomotion and the enhanced dorsal root reflex in disinhibited lumbar locomotor networks are resistant to ADO. Because ADO effects in standard solution occurred at doses that are notably higher than those occurring in vivo, we hypothesize that newborn rat locomotor networks are rather insensitive to this neuromodulator.	{ "pile_set_name": "PubMed Abstracts" }
Clinical profiles of four large pedigrees with familial dilated cardiomyopathy: preliminary recommendations for clinical practice. This study aimed to characterize the clinical profile of familial dilated cardiomyopathy (FDC) in the families of four index patients initially diagnosed with idiopathic dilated cardiomyopathy (IDC) and to provide clinical practice recommendations for physicians dealing with these diseases. Recent evidence indicates that approximately one-half of patients diagnosed with IDC will have FDC, a genetically transmissible disease, but the clinical profile of families screened for FDC in the U.S. has not been well documented. Additionally, recent ethical guidelines suggest increased responsibilities in caring for patients with newly found genetic cardiovascular disease. After identification of four families with FDC, we undertook clinical screening including medical history, physical examination, electrocardiogram and echocardiogram. Diagnostic criteria for FDC-affected status of asymptomatic family members was based on left ventricular enlargement (LVE). Subjects with confounding cardiovascular diagnoses or body mass indices >35 were excluded. We identified 798 living members from the four FDC pedigrees, and screened 216 adults and 129 children (age <16 years). Twenty percent of family members were found to be affected with FDC; 82.8% of those affected were asymptomatic. All four pedigrees demonstrated autosomal dominant patterns of inheritance. The average left ventricular end-diastolic dimension was 61.4 mm for affected and 48.4 mm for unaffected subjects, with an average age of 38.3 years (+/- 14.6 years) for affected and 32.1 years for unaffected subjects. The age of onset for FDC varied considerably between and within families. Presenting symptoms when present were decompensated heart failure or sudden death. We propose that with a new diagnosis of IDC, a thorough family history for FDC should be obtained, followed by echocardiographic-based screening of first-degree relatives for LVE, assuming their voluntary participation. If a diagnosis of FDC is established, we suggest further screening of first-degree relatives, and all subjects with FDC undergo medical treatment following established guidelines. Counseling of family members should emphasize the heritable nature of the disease, the age-dependent penetrance and the unpredictable clinical course.	{ "pile_set_name": "PubMed Abstracts" }
Q: Why do you need excess LAH to reduce esters? I am little confused on this question. On one hand, I remember my teacher saying that $\ce{LiAlH4}$ is like $\ce{BH3}$ of hydroboration oxidation of alkene, where you one mole of $\ce{BH3}$ can oxidize 3 mole of alkene molecule. but on the other hand my textbook keeps on mentioning excess LAH when reducing ester? Can't one mole of LAH reduce four mole of ester molecules as well? Thanks. A: Lithium aluminium hydride or LAH is the more everyday form of $\ce{LiAlH4}$. When originally produced, most of it is indeed $\ce{LiAlH4}$ but that quickly partially hydrolyses giving the grey powder you may or may not know from the lab. As such, $\ce{LiAlH4}$ is practically never entered into reactions in pure form. Since it is impure, excess reagent is added to make sure the reduction job is performed as desired. Also, remember to consider the reaction meachnism: $$\ce{R-COOR' ->[LAH][- HOR'] R-CHO ->[LAH] R-CH2OH}\tag{1}$$ Note that the second step, the reduction of an aldehyde, is more rapid than the first as aldehydes are more reactive towards nucleophiles than esters. Thus, if you attempted to bargain, hoping to arrive at the aldehyde selectively, you would end up with under half of your reactant reduced to the alcohol and half of it still as an ester. Another reason to always add excess just to be sure.	{ "pile_set_name": "StackExchange" }
Karen Bleier/AFP/Getty Images A single unit of Bitcoin, the volatile digital currency that most people have never actually used, hit an all-time high Thursday, making it more valuable than an ounce of gold. The exchange price for one bitcoin rose $33.36 to $1,263.72, an increase of 2.7 percent, according to CoindDesk's bitcoin price index. Meanwhile, an ounce of gold was trading up $1.70 to $1,233.30. Since the beginning of the year, bitcoin's value has risen more than 25 percent, while gold is up a little more than 7 percent. Since its founding in 2009, bitcoin has made a name for itself by allowing for anonymous transactions. The digital currency is now accepted by more than 100,000 merchants worldwide, including Microsoft, Dish and Subway. But bitcoin's lack of government backing and regulation has led to volatility. Its ever skyrocketing valuation a few years back attracted investors, but some of that enthusiasm faded after bitcoin exchange Mt. Gox declared bankruptcy in 2014 following the reported theft of almost 750,000 customer bitcoins. The value of bitcoin plummeted in August 2016 after a hacker managed to steal millions of dollars worth of the digital currency. Experts suggest the growth corresponds with a weakening in the Chinese yuan; bitcoin is apparently attractive to Chinese traders because it enables them to evade currency controls. Virtual reality 101: CNET tells you everything you need to know about what VR is and how it'll affect your life. Batteries Not Included: The CNET team shares experiences that remind us why tech stuff is cool.	{ "pile_set_name": "OpenWebText2" }
Introduction {#sec1-1} ============ Nidanas (etiological factors) are the agents responsible for the causation of any disease -- be it directly or indirectly. Ayurveda has laid down the importance of these etiological factors for both the causation of the disease and the treatment for the avoidance of the Nidanas. A list of various Nidanas\[[@ref1]\] have been given in the texts for every disease as well as for all stages of the pathogenesis. In the chapter of Pandu Roga, Acharya Charaka has described various psychological etiological factors as Kama (excessive thinking about sex), Krodha (anger), Chinta (excessive worrying), Bhaya (fear) and Shoka (grief).\[[@ref1]\] However till now, no scientific study describing the mechanism of these factors in the causation of anemia has been reported. Hence, it was decided to study the three factors Chinta, Bhaya and Shoka which are collectively called as the main causes of psychological stress (PS) which in turn play a crucial role in the causation of various anemia and to observe the findings for any explanations. Review of modern science literature and researches {#sec1-2} -------------------------------------------------- A thorough search was made on the search engine Google, Bing and PubMed, regarding the topic using the keywords -- role of PS in the causation of any anemia and its mechanisms. Results {#sec1-3} ======= A few scientific studies were found describing the role of PS in the causation of iron deficiency anemia. The first study\[[@ref2]\] (conducted in the Department of Naval Medicine, Second Military Medical University, Shanghai) performed in an animal model of twenty male Sprague-Dawley rats in whom PS was induced through a communication box. A communication box was divided into room A and room B with a transparent acrylic board, room A included ten little rooms with a plastic board-covered floor and room B included ten little rooms with a metal grid-exposed floor for electric insulation. Rats in room B were randomly given electrical shock 90 V, 0.8 mA for 1 s for 30 min, 60 times in total through the floor and exhibited no receptive stimulation-evoked responses, such as jumping up, defecation, and crying. Rats in room A were only exposed to the responses of rats in room B to establish PS model. On the 7^th^ and the 14^th^ day after administration, ten rats were executed and the rat blood and femoral bone marrow were collected for analysis of serum iron (SI), serum ferritin (SF), serum transferrin receptors, hemoglobin (Hb), red blood cell (RBC) count, RBC distribution width (RDW), mean corpuscular volume (MCV), serum erythropoietin (EPO) and bone marrow iron. Experimental data were statistically analyzed with SPSS 11.0. The data revealed that for rats analyzed on the 7^th^ and 14^th^ day in PS group, the following points were noted. Femoral bone marrow iron was significantly decreasedSI was decreased by 28.6% (P \< 0.01) and 27.5% (P \< 0.01)Hb was decreased by 10.0% (P \< 0.01) and 12.8% (P \< 0.01)RBC count was decreased by 5.1% (P \< 0.05) and 9.8% (P \< 0.01)MCV was decreased by 1.7% (P \< 0.05) and 7.3% (P \< 0.01)RDW was increased by 10.7 and 22.5%SF, transferrin receptor and EPO showed no significant changes in comparison with controls after 7^th^ day of administration, but SF and EPO were decreased by 23.8 and 12.3% while transferrin receptor increased by 31.5% after 14^th^ day of administration. Another study conducted at the same place but by other workers\[[@ref3]\] further confirmed the above findings and also described the mechanism responsible for it as the interleukin-6 (IL6) hepcidin axis. This study was also an experimental study in rats done in the same way as stated above through a communication box. The investigators found that the SI level was decreased after 3 day repeated PS exposure before the decline of red cell count and Hb (which decreased on 7^th^ day). They also noticed elevated body iron stores in those rats as elevated hepatic iron concentration indicating that PS changed the iron distribution of the body and limited the transportation and utilization of iron. Only male rats were included in the study and standard diet was given to the rats to exclude the factors related to feeding loss and menstrual blood. The researchers also noticed increased IL6 after repeated PS exposure which was through the activation of the hypothalamic-pituitary-adrenal (HPA) axis and sympathetic nervous system. They also observed the up-regulation of hepcidin and down-regulation of ferroportin through the Western blot technique after PS exposure. The investigators further performed anti IL6 antibody experiments to examine whether the IL6-hepcidin axis was necessary for the development of hypoferremia induced by PS. They found that anti-IL6 antibody inhibited the up-regulation of hepcidin and down-regulation of ferroportin while also inhibiting liver and SI level changes. Another experimental study conducted on rats in the Department of Pathology,\[[@ref4]\] University of Pittsburgh School of Medicine, Pennsylvania, also had similar findings of elevation of plasma IL6 on exposure to physical and psychological stressors which they further related to the activation of HPA axis. Discussion {#sec1-4} ========== Although Chinta, Bhaya and Shoka (PS) are described as etiological factors in the causation of Pandu Roga in Ayurveda\[[@ref5]\] but no detail about the exact mechanism of action and the pathological process has been made there. However, at certain places, some specific hints are obtained which clarify and elaborate the whole understanding about the topic. An important aspect about the association between these psychological factors and Pandu Roga is a direct cause and effect relationship as excessive worry or stress (Chintyaanam cha Atichintanaat) has been described as the specific etiological factor for the vitiation of Rasa Vaha Srotas\[[@ref6]\] (channels carrying the first tissue element of the body formed from the digested nutrients) and Pandu Roga is a Rasa Pradoshaja Vikara.\[[@ref7][@ref8]\] Yet, it is clearly understood that certainly there must be several steps or processes between these two extreme points of cause and effect. These missing links are in the form of Agni vitiation. References are available in the texts which state that\[[@ref9][@ref10][@ref11]\] wholesome food taken even in the right quantity does not get digested properly if the individual is afflicted with grief, fear, anger, sorrow and inconvenient bed for sleep (meaning disturbed sleep) infering thereby that these factors vitiate Agni and resultantly the digestion process. In Ayurveda, the concept of digestion (Pachana) relates to the whole process of digestion, metabolism, absorption and assimilation in the body and depends on the proper functioning of the Agni.\[[@ref12]\] It is only after the digestion by Jatharagni and Bhutagni that the food substrate gets converted into a form suitable for use by our body tissues and gets converted into the respective tissue by the action of the respective Dhatvagnis.\[[@ref13]\] All these Bhutagnis and Dhatvagnis depend upon the main Agni, i.e., Jatharagni for their nourishment and strength. Vitiation of Jatharagni will also vitiate the other Agnis in due course of time and ultimately affect the status of tissues in the body. Thus, this improper digestion might be related to any of the aspects stated above, resulting in the deficient production of Rasa Dhatu from Adya Rasa Dhatu (the fluid tissue of the body which contains the end products of digestion and metabolism and circulates it in the whole body for nourishing other body tissues) either quantity-wise or quality-wise (deficiency in the amount of nutrients present in it as result of digestion and absorption). This improper Rasa Dhatu further effects the production of Rakta Dhatu (which is produced by the action of Raktagni on Rasa Dhatu)\[[@ref14]\] This could be the reason why the Acharyas have included Pandu in Rasa Pradoshaja Vikaras and described Alpa Rakto (decreased blood) as one of the main features of the disease along with Panduta.\[[@ref15]\] Besides the above-stated processes, PS also has some other impacts on the body, for it is one of the factors responsible as an etiological agent for generalized debilitation of the body (Samanya Kshaya Hetu)\[[@ref16]\] as well as for decreased strength and immunity status of the body (Oja Kshaya).\[[@ref17]\] It is worthwhile mentioning here that in the disease Pandu Roga also, there is description of decrease in the qualities of the Ojas (Ojo Guna Kshaya)\[[@ref18]\] and absence of pure essence in all the body tissues (Nihsaarata). Ayurveda states that the entity responsible for the intellectual capacities of the individual, enthusiasm, pride, the achievement of determined goals -- all depends upon Sadhaka Pitta, which is located in the Hridaya.\[[@ref19]\] The pathogenesis of Pandu Roga also describes the involvement of Hridyastha Pitta in the disease pathogenesis.\[[@ref5]\] Hence, certainly, there is involvement of Sadhaka Pitta also by the effect of PS. It is also important to recall here that Rasa Dhatu is also the seat of Pitta Dosha.\[[@ref20]\] Hence, covering all the above-stated aspects regarding impact of PS, the following pathogenesis is proposed \[[Figure 1](#F1){ref-type="fig"}\]. ![The pathogenesis of psychological stress in causing Pandu Roga and its effects in the body](AYU-37-18-g001){#F1} The scientific description provided by the studies quoted above specifies that the PS continued even for a small period of 7 -- 14 days, changes iron distribution within the body and limits the transportation and utilization of iron; thereby causing a significant reduction of SI and bone marrow iron, significant inhibition of erythropoiesis process,\[[@ref21]\] and an increase in the body iron stores (as hepatic iron concentration increased).\[[@ref22]\] This process is mediated by the increased production of IL6 through the activation of the HPA axis and sympathetic nervous system. It is also to be noted here that the pituitary and the adrenal glands are capable of producing IL6,\[[@ref22]\] which may also function as a hormone to induce the production of acute phase proteins from the hepatocytes\[[@ref23]\] and to regulate the secretion of hormones from the hypothalamus as well as the pituitary and adrenal glands.\[[@ref24][@ref25]\] IL6 has been shown to stimulate the hepcidin expression in vitro and in vivo:\[[@ref26]\] which may be the mechanism responsible here also for the up regulation of hepcidin, collectively leading to the hypoferremia and hepatic iron storage. This increase of IL6 and hepcidin by the PS resulting in iron deficiency anemia through various mechanisms is quite consistent with the Ayurveda description pertaining to Pandu Roga and Agni. This also correlates to some extent to the description of Ayurveda pathogenesis of Pandu Roga (Samprapti) which states that Pandu Roga is a Pitta Pradhana Vyadhi (IL-6 and hepcidin are considered in the modern medical science as inflammatory mediators) and Rasa Pradoshaja Vikara. The above descriptions have clearly shown that Rasa Dhatu is getting affected here and is then causing Pandu Roga. The increase of IL6 and hepcidin which are regulatory proteins also acting as hormones is quite similar to the increase of Pitta (as they have functions similar to that of Pitta). This vitiated Pitta then circulates in the whole body by the channels of circulation or Srotasa getting lodged in the Rasa Dhatu and results in the manifestation of Pandu Roga. Initially, only the Rasa-Vaha Srotasa (channels) are involved, but later, all the tissues of the body and their channels might also be involved, that is why features such as Nihsaarata and Ojo Kshaya Lakshanas (features) are present in the patient, resulting in his/her decreased strength, work capacity and immunity status of the individual (described as Bala/Oja in Ayurveda). Conclusion {#sec1-5} ========== The above-stated studies and the discussion reveals that the scientific explanation to the etiopathogenesis of Chinta, Shoka and Bhaya in the causation of Pandu Roga, i.e. to say that these factors cause iron deficiency anemia by causing a significant reduction of serum and bone marrow iron while also inhibiting the process of erythropoiesis. This study also reveals the involvement of inflammatory mediators such as IL6, hepcidin in the pathogenesis of Pandu Roga caused due to the above-stated factors of Shoka and Bhaya, which have been described to be Vata dominant. Earlier studies have already proven that the inflammatory mediators are very much similar to the Pitta Dosha of Ayurveda. Thus, the above study throws some light on the possible role of pitta in the pathogenesis of Pandu Roga and confirms the Ayurveda Samprapti also to some extent. However, still more studies are required to throw light on the other attributes of the pathogenesis of Pandu Roga. Financial support and sponsorship {#sec2-1} --------------------------------- Nil. Conflicts of interest {#sec2-2} --------------------- There are no conflicts of interest.	{ "pile_set_name": "PubMed Central" }
Countercurrent liquid-liquid extraction on paper. Proof-of-concept is shown for two-phase countercurrent flow on paper. The device consists of two paper layers, one of which has been modified with a sizing agent to be hydrophobic. The layers exhibit different wetting behavior for water and octanol. Both phases dominate wetting in one of the layers and can be made to move in different directions along the interface to achieve liquid-liquid extraction.	{ "pile_set_name": "PubMed Abstracts" }
Q: Converting a row of a pandas dataframe into a dataframe itself (instead of a series)? I have a df that I'm iterating over, like so for _, row in df.iterrows(): process(row) The function process takes the argument and itself does an iterrows() on it. It does this because it is normally passed a dataframe. However, I'd like to pass a single row to process and still have it function normally. The problem is that row is a Series, and not a dataframe. And Series can not be iterated over with an .iterrows() method. I tried converting the row to a dataframe like so row = row.to_frame() but that doesn't seem to preserve the indices, columns, etc. Is there a way to do this easily? Or should I re-write the process function to be able to handle a single Series/row? A: You can transpose the output of to_frame: s.to_frame().T That said, this seems a strange thing to require, a refactor of process may be a good idea. But perhaps you can get away with chunkifying into smaller dataframes: for chunk in np.array_split(df, 50): # 50 chunks process(chunk)	{ "pile_set_name": "StackExchange" }
Brian Fallon has released his brand new track If Your Prayers Don’t Get To Heaven. It’s been taken from the The Gaslight Anthem vocalist’s upcoming solo album Sleepwalkers, which will arrive on February 9 via Virgin EMI. Fallon previously shared the song Forget Me Not back in October. Speaking about If Your Prayers Don’t Get To Heaven, Fallon says: “I took a Motown beat and some fingerstyle guitar and wrote a letter for the times when we feel like our prayers and dreams seem to hit nothing but ceilings. When really, they’re being looked after by our loved ones until they leave the waiting room.” Fallon will head out on a European tour with his band The Howling Weather throughout February and March in support of Sleepwalkers, which is now available for pre-order. Find further details below. Brian Fallon Sleepwalkers tracklist If Your Prayers Don’t Get To Heaven Forget Me Not Come Wander With Me Etta James Her Majesty’s Service Proof Of Life Little Nightmares Sleepwalkers My Name Is The Night Neptune Watson See you On The Other Side Feb 20: Birmingham O2 Institute, UK Feb 21: Manchester O2 Ritz, UK Feb 22: Glasgow O2 ABC, UK Feb 23: London Koko, UK Feb 24: Nottingham Rock City, UK Feb 25: Bristol SWX, UK Feb 27: Antwerp De Roma, Belgium Feb 28: Cologne Live Music Hall, Germany Mar 01: Berlin Astra, Germany Mar 02: Vienna Arena, Austria Mar 03: Nürnberg Löwensaal, Germany Mar 04: Munich Theaterfabrik, Germany Mar 06: Amsterdam Melkweg, Netherlands Mar 08: Newcastle Boiler Shop, UK Mar 09: Leeds Beckett, UK Mar 10: Dublin Olympia Theatre, Ireland Mar 11: Belfast Limelight, UK My life in 10 songs by Brian Fallon	{ "pile_set_name": "OpenWebText2" }
537 U.S. 1045 WILD ET UX.v.SUBSCRIPTIONS PLUS, INC., ET AL. No. 02-316. Supreme Court of United States. December 2, 2002. 1 CERTIORARI TO THE UNITED STATES COURT OF APPEALS FOR THE SEVENTH CIRCUIT. 2 C. A. 7th Cir. Certiorari denied. Reported below: 292 F. 3d 526.	{ "pile_set_name": "FreeLaw" }
Hmm.... On avast's website they say that Sandboxing is Pro and up but what is auto sandbox? Hmm.. I can only tell you that I have the free version and you see the screenshot; yes? The best way I can describe it in layman's terms is that Avast 8 is monitoring all PC activity; period. The nice thing I like about Avast is you can tell when its working because the animated icon in the system tray starts to spin. Anyway, it not only monitors for malware but it also monitors for any suspicious program activity that cannot be positively identified as malware but appears to be executing in a very suspicious manner. If identified as such, the program will be placed in a sandbox environment until it can be fully analyzed by Avast. Once done, recommendations will follow. This is very useful when a brand new virus surfaces and virus definitions have not been updated to positively identify the malware. Let's discuss apps, YOUR personal favorites that you've come across. My personal favorite that I adore, Cocktail Flow. :cool: It's absolutely well done in the metro form and just FANTASTIC! There are SO many drinks.... WOW! :dinesh: I have two favorites, the Video app and the Mail app. Whenever I go back to my Windows 7 Ultimate partition for some reason I miss these two apps so much! I now simply cannot live without at least the Mail App, it's incredibly simple and at the same time so handy and practical. Having to open up my... Ok, after a clean install, what are the first must do tweaks you do? EDIT: Thanks for all of the input so far. Keep them coming! Here's a quick list from me. - Disable UAC (Never Notify) - Disable All Notification Center Notices - Netplwiz - Disable Firewall and Defender - Disable System... THIS POST HAS BEEN MOVED! VISIT THE NEW ONE HERE Welcome! Please take the survey here: bit.ly/1eL9nJF. The survey ends on the 31st of March and the results will be published here (photos of the graphs and a Microsoft Excel file). UPDATE 1/10/2014: The survey is open! View it here!...	{ "pile_set_name": "Pile-CC" }
Q: Grant access for any logged in user for common database In SQL server 2008, I have one database that is a common database that is accessed thru stored procedures in all other databases. Each of the other databases have their own login. I need a way that all logged in users can access that common database. I know I could create a user for the common database for each login but I would need to create over 100 users in the database then. Is there a better way? A: I believe you can create a user account in that database, using WITHOUT LOGIN. This will create it where you can grant execute as permissions to the other users for any particular stored procedure in that common database. They don't have to use a password for it so you control it by who can EXECUTE AS with it. Here is a pretty good write-up on how it could be used, near the end he talks on how it can be used outside the context of the database.	{ "pile_set_name": "StackExchange" }
The fire still burns in his belly, which is why we'll see those belly rolls again in 2019. Brandon Mebane put pen-to-paper Wednesday afternoon on a two-year deal to remain a Los Angeles Charger. Truth be told, Mebane wasn't sure he'd be back. After 12 years in the league, and a draining personal tragedy in which his infant daughter passed away after being born premature, the 34-year old took a few weeks off before making a decision. "I took a month or two to see if the desire was still there, and it is," he explained. "So I talked to my wife, and she said if the fire is still there, go get it. You have to have that desire to play this game. It's something that's just in you. I just love the game. I love playing. I love competition. And it's needed because at some point, money doesn't motivate. The money is going to be there. You still have to perform at some point. And what motivates me is family. That's major. It's key. I'm just doing it for them. Seeing them going to the games and in stands, it's an (incredible) feeling." When discussing his desire to play, Mebane routinely brings up his family. He's also quick to discuss his daughter, Makenna, who passed away weeks after being born premature with trisomy 13. "If she would have made it out of her situation, I probably wouldn't be playing this year because we would have had to do a lot of therapy," Mebane said. "She's definitely still in my heart. I'm definitely going to miss her. Now, my oldest kid is about to turn five in April and my youngest, three in May. It's exciting because my kids are getting to the age now where they're starting to understand what I do for a living. They go to school, and they tell kids at school, 'My daddy plays football.' That's exciting. That's fun." Meanwhile, once Mebane decided to keep playing, there was only one team he wanted to play for. In fact, he didn't even bother paying any mind to interest from other teams. "The Chargers mean a lot to me" he said. "I spent my previous three years here, and I like the organization. I like the direction that we're going, and I wanted to be a part of this system that I'm very familiar with. I've (been in it) pretty much since my rookie year. I didn't want to go anywhere else." Thus, in the end, returning to the Chargers to play his 13th NFL season was an easy to decision. And, as if those reasons weren't enough, the moves the Bolts made early in free agency have also further stoked his flames. More specifically, he's pumped over the addition of veteran linebacker Thomas Davis. In fact, Mebane burst out into one of his patented gut-busting laughs when talking about his newest teammate.	{ "pile_set_name": "OpenWebText2" }
Q: "The decimal field must be a number" I'm trying to find a possible easy solution for this issue. All the solutions found in web are not working for me. I have in my model a price field which can be a decimal value like 30,5 using comma. But the validation returns me an error "The 'field' must be a number". I'm using the default validation used in MVC that I suppose it is using jQuery. Is there any way to avoid this issue? The model code is: [Range(0.0, Double.MaxValue, ErrorMessage = "Out of range")] [DataType(DataType.Currency)] public decimal Price { get; set; } A: I believe the error is coming from client-side validation, not server-side. If it actually got to the server, you should be fine having the culture specified. However, ASP.NET's unobtrusive validation actually use the jQuery Validation plugin, and as you can see here at the documentation page for the number validator, only a . as the decimal separator will validate. You may simply have to remove the number validation rule from the field. $("#Price").rules("remove", "number"); UPDATE This post may help you: http://blog.icanmakethiswork.io/2012/09/globalize-and-jquery-validate.html. It explains how to essentially monkey-patch jQuery Validation to actually pay attention to culture.	{ "pile_set_name": "StackExchange" }
Q: Load Facebook into an iframe I can't load facebook into an iframe, in a web page like the following one: <html> <head> <!-- some stuffs here --> </head> <body> <!-- some stuffs here --> <iframe src="http://www.google.com" frameborder="0"> </iframe> </body> </html> I've tested it with other websites and it seems to load without problems for instance for wired.com, but not for facebook.com... Can anyone explain me why? I'm using Google Chrome and Safari, if needed. It seems to be as if Google blocks iframe loading of its page. A: If you use Firebug or Google Chrome's developer console, you can see the following error Refused to display document because display forbidden by X-Frame-Options. X-Frame-Options DENY The page cannot be displayed in a frame, regardless of the site attempting to do so. SAMEORIGIN The page can only be displayed in a frame on the same origin as the page itself. Here is another related stackoverflow question Overcoming “Display forbidden by X-Frame-Options” A: Google and Facebook are using a X-Frame-Options in the HTTP response header to avoid the content being loaded in a iFrame. The X-Frame-Options HTTP response header can be used to indicate whether or not a browser should be allowed to render a page in a or . Sites can use this to avoid clickjacking attacks, by ensuring that their content is not embedded into other sites. Source: https://developer.mozilla.org/en/The_X-FRAME-OPTIONS_response_header I don't think it is possible for you to override this setting.	{ "pile_set_name": "StackExchange" }
[Anatomo-surgical notes on transhiatal access in esophagectomy]. The Authors through an anatomic study on 20 cadavers specify the surgical procedure for transhiatal esophagectomy and describe the anatomical structures involved. The proper manoeuvres and artifices to avoid intraoperative accidents are suggested. Finally, the indications for this peculiar operation are discussed.	{ "pile_set_name": "PubMed Abstracts" }
Independence Museum of Azerbaijan The Independence Museum of Azerbaijan or "Istiqlal" Museum () – is a museum established on 7 December 1919 in Baku - the capital of the Azerbaijan Democratic Republic. H. Mirzajamalov and I. M. Aghaoglu had a great role in creation of the museum. Archeological finds, exemplars of rare books, objects of numismatics, jewelry, etc. were collected in the museum. The museum was located in the building of the ADR’s Parliament (at present – the building of the Institute of Manuscripts of Azerbaijan National Academy of Sciences). It is noted that, namely at that time, an attempt at making a legal document about organizing and storing museum items was undertaken. The museum existed only a year and couldn’t realize all intended plans. It was liquidated in 1920, when the Soviet Power was established in Baku. Materials collected in the museum became basis for "Muzexcurs" foundations and Azerbaijan State Museum. The second Independence Museum was established on 9 January 1991. Then the museum had only 7,000 exhibits. Due to attempts and investigations of the museum's collective the number of exhibits is above 20,000 now. The main goal of the museum is to highlight national independence movement of Azerbaijan that lasts from ancient times till now. The exposition of the museum is exhibited in six halls: The first hall is dedicated to the history of Azerbaijan from the ancient times to the 19th century, the second hall to the history of Azerbaijan between the second half of the 19th and 20th centuries, the third hall to national independence movement in the Southern Azerbaijan in the first half of the 20th century, the fourth hall to the history of Azerbaijan during repression and the Great Patriotic War, the fifth hall to national independence movement of Azerbaijan at the end of the 20th century and Karabakh War, and the sixth hall to the history of Independent Republic of Azerbaijan and activity of the national leader Heydar Aliyev. There are masterpieces of art and architecture, maps, pictures, books, currencies and other exhibits in the Independence Museum of Azerbaijan. A lot of expositions and activities dedicated to historical events are held in the exposition of the museum. The museum opens its doors during such events as the International Day for Monuments and Sites (April 18), International Museum Day (May 18) and World Tourism Day (September 27). Free access to the museum is available for members of ICOM (International Council of Museums), museum workers, military personnel, veterans of World War II, victims of the Karabakh war and Black January. The museum also has a children’s circle called “We are the heirs of the independence”, where children are offered a variety of tasks and told about the history of the state in entertaining form. References Category:Museums in Baku Category:1919 establishments in Azerbaijan Category:Museums established in 1919	{ "pile_set_name": "Wikipedia (en)" }
Q: Can .NET Ria service push data from server to client? The question has been asked previously for Silverlight 3.0 but now that Silverlight 4 is out and Silverlight 5 is on the horizon, is it possible to push data from server to client with RIA services yet? A: Not yet. You can watch the Wish List for updates.	{ "pile_set_name": "StackExchange" }

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