text:
\section*{\sc \bf Supplemental Material}
\subsection{Steady-state solution}
\label{app:solution}

In this section we briefly detail the solution for the non-equilibrium steady state using the quantum Langevin formalism. We consider a general quadratic Hamiltonian of the form $\hat{H}_{\rm tot} = \hat{H}_S + \hat{H}_{SB} + \hat{H}_B$, with
\begin{align}\label{H_S}
	\hat{H}_S  & = \sum_{j,k} H_{jk} \ensuremath{\hat{a}^\dagger}_j\a_k, \\
	\label{H_SB}
	\hat{H}_{SB} & = \sum_{j\in \partial S} \sum_q g_{qj} \left (\ensuremath{\hat{a}^\dagger}_j \b_{qj} + \ensuremath{\hat{b}^\dagger}_{qj} \a_j \right ), \\
	\label{H_B}
	\hat{H}_B & =  \sum_{j\in \partial S} \sum_q \Omega_{qj} \ensuremath{\hat{b}^\dagger}_{qj} \b_{qj}.
\end{align}
In Eq.~\eqref{H_S}, $\a^\dagger_j$ creates a boson or fermion on site $j$ of the system and $H_{jk}$ are the elements of a hermitian single-particle Hamiltonian matrix, $\mathbf{H}$. Similarly, the canonical operators $\ensuremath{\hat{b}^\dagger}_{qj}$ create a particle in mode $q$ of the reservoir connected to site $j$, with corresponding frequency $\Omega_{qj}$ and coupling $g_{qj}$ to a site $j$ lying on the boundary of the system, $\partial S$.

Following the standard procedure, we formally solve the equations of motion for $\b_{qj}$ in the Heisenberg picture and substitute the result into the Heisenberg equation for $\a_j$, obtaining
\begin{equation}\label{QLE_general}
	\ensuremath{\mathrm{i}} \partial_t\hat{a}_j(t) =  \sum_k H_{jk} \a_k(t) + \int_{t_0}^\infty\mathrm{d} t'\, \chi_j(t-t') \a_j(t') + \hat{\xi}_j(t).
\end{equation}
Above, we have introduced the retarded memory kernel $\chi_j(t)$ and the noise operator $\hat{\xi}_j(t)$, which for $j\in \partial S$ are given by
\begin{align}
	\label{noise_op}
	\hat{\xi}_j(t) & = \sum_q g_{qj} \ensuremath{\mathrm{e}}^{-\ensuremath{\mathrm{i}} \Omega_{qj}(t-t_0)} \b_{qj}(t_0), \\
	\label{memory_kernel}
	\chi_j(t) & = -\ensuremath{\mathrm{i}} \theta(t)\sum_q g^2_{qj} \ensuremath{\mathrm{e}}^{-\ensuremath{\mathrm{i}} \Omega_{qj}t},
\end{align}
with $\theta(t)$ the unit step function, while for $j\notin \partial S$ we define $	\hat{\xi}_j(t) = 0 = \chi_j(t) $. Note that the memory kernel is nothing but the retarded Green function of the noise operator, since $\theta(t-t')\langle [\hat{\xi}_j(t),\hat{\xi}^\dagger_k(t')]_\pm\rangle = \ensuremath{\mathrm{i}}  \delta_{jk}\chi_j(t-t')$, where the minus (plus) sign indicates the (anti-)commutator for bosons (fermions).

Since we are interested in the steady state, we take the limit $t_0\to -\infty$ in Eq.~\eqref{QLE_general} and solve in the Fourier domain. The solution can be expressed in the compact form
\begin{equation}\label{a_solution_vector}
	\tilde{\mathbf{a}}(\omega) = \mathbf{G}(\omega) \cdot \tilde{\boldsymbol{\xi}}(\omega),
\end{equation}
by defining vectors $\tilde{\mathbf{a}}= (\tilde{a}_1, \tilde{a}_2,\ldots  )^T$ and $\tilde{\bm{\xi}}(\omega) = (\tilde{\xi}_1, \tilde{\xi}_2,\ldots  )^T$ of Fourier-transformed operators and introducing the (matrix-valued) retarded Green function
\begin{equation}\label{G_ret}
	\mathbf{G}(\omega) = \left [ \omega\mathbf{1} - \mathbf{H} -\mathbf{\Sigma}(\omega) \right ]^{-1}.
\end{equation}
Here, $\mathbf{1}$ is the identity matrix and the retarded self-energy matrix $\mathbf{\Sigma}(\omega)$ is diagonal with elements $\Sigma_{jk}(\omega) = \delta_{jk} \tilde{\chi}_j(\omega)$ given by the Fourier transform of the memory kernel. The latter decomposes as
\begin{equation}\label{memory_kernel_decomp}
	\tilde{\chi}_j(\omega) = \fint \frac{\mathrm{d}\omega'}{2\pi} \frac{\gamma_j(\omega')}{\omega-\omega'} - \ensuremath{\mathrm{i}} \frac{\gamma_j(\omega)}{2},
\end{equation}
where $ \fint$ denotes a principal-value integral and we introduced the spectral density
\begin{equation}\label{spectral_density}
	\gamma_j(\omega) = 2\pi \sum_q g_{qj}^2\delta(\omega-\Omega_{qj}).
\end{equation}

The non-equilibrium steady state of the system depends on the statistical properties of the noise operator via Eq.~\eqref{a_solution_vector}. Assuming that the initial state of the reservoirs (at time $t=t_0$) is thermal and uncorrelated, we find the noise spectrum
\begin{equation}\label{noise_spectrum}
	\langle \tilde{\xi}^\dagger_j(\omega) \tilde{\xi}_k(\omega')\rangle = 2\pi\delta(\omega-\omega')\delta_{jk} \gamma_j(\omega) f_j(\omega),
\end{equation}
where $f_j(\omega) = (\ensuremath{\mathrm{e}}^{\beta_j(\omega-\mu_j)} \pm 1 )^{-1}$ is the reservoir distribution function, characterized by an inverse temperature $\beta_j$ and chemical potential $\mu_j$, and expectation values are taken with respect to the state at time $t=t_0$. It is now straightforward to write down the two-point correlation function of the system in its steady state, $C_{jk}(t) = \langle \ensuremath{\hat{a}^\dagger}_k(t) \a_j(0)\rangle$, as
\begin{equation}\label{two_point_function}
	\mathbf{C}(t) = \int\frac{\mathrm{d}\omega	}{2\pi} \ensuremath{\mathrm{e}}^{\ensuremath{\mathrm{i}}\omega t} \mathbf{G} \cdot (\mathbf{\Gamma} \circ \mathbf{F}) \cdot \mathbf{G}^\dagger.
\end{equation}
Here we have suppressed frequency arguments and defined diagonal matrices $\mathbf{\Gamma} = \ensuremath{\mathrm{i}} (\mathbf{\Sigma} - \mathbf{\Sigma}^\dagger)$ and $F_{jk} = \delta_{jk} f_j$, while $\circ$ denotes the elementwise (Hadamard) product. The steady-state correlation matrix $\mathbf{C} = \mathbf{C}(0)$ is found simply by setting $t=0$ in Eq.~\eqref{two_point_function}.

The setup considered in the main text features hot baths coupled to sites on the boundary at $x=1$ and cold baths coupled to the other boundary at $x=L_X$. Moreover, the wide-band limit approximation is made, which amounts to replacing the spectral densities $\gamma_j(\omega)$ by frequency-independent constants. This approximation is valid so long as $\gamma_j(\omega)$ does not vary significantly over the frequency range within which the integrand of Eq.~\eqref{two_point_function} differs appreciably from zero.  Assuming symmetric coupling, $\gamma_j = \gamma$, one then recovers Eq.~(4). In this case, $\mathbf{\Gamma} = \mathbf{\Gamma}_h + \mathbf{\Gamma}_c$, where the self-energy $\mathbf{\Gamma}_h$ ($\mathbf{\Gamma}_c$) of the hot (cold) bath is given by a diagonal matrix, with $[\mathbf{\Gamma}_{h,c}]_{jk} = \gamma \delta_{jk}$ whenever $j$ corresponds to a boundary site with $x=1$ ($x=L_X$) and $[\mathbf{\Gamma}_{h,c}]_{jk} = 0$  otherwise. Likewise, we have $f_j = \bar{n}_h$ ($f_j = \bar{n}_c$) for $j$ corresponding to $x=1$ ($x=L_X$).

\subsection{Definition of currents}
\label{app:currents}

The current densities are defined via the continuity equation for the particle density, $\hat{n}_{x,y} = {\bf\a}^\dagger_{x,y}
\cdot {\bf \a}_{x,y}$, as
\begin{align}\label{continuity_equations}
	\ensuremath{\mathrm{i}} [\hat{H}_X, \hat{n}_{x,y}] & = \hat{J}^X_{x-1,y} - \hat{J}^X_{x,y} \notag \\
	\ensuremath{\mathrm{i}} [\hat{H}_Y, \hat{n}_{x,y}] 	& =  \hat{J}^Y_{x,y-1} - \hat{J}^Y_{x,y}.
\end{align}
Here $\hat{J}^X_{x,y}$ denotes the current density operator describing particle flow from site $(x,y)$ to its nearest neighbour in the $x$ direction, i.e.~$(x,y) \to (x+1,y)$. Similarly, $\hat{J}^Y_{x,y}$ is the corresponding current in the $y$ direction, $(x,y) \to (x,y+1)$. Using the canonical (anti-)commutation relations, it is straightforward to derive
\begin{align}
	\label{current_op_X}
	\hat{J}^X_{x,y} & = \frac{t_X}{2\ensuremath{\mathrm{i}} } {\bf \a}^\dagger_{x+1,y}\cdot (\sigma_z+\ensuremath{\mathrm{i}}\sigma_y)\cdot {\bf \a}_{x,y} + {\rm h.c.},\\
	\label{current_op_Y}
	\hat{J}^Y_{x,y} & = \frac{t_Y}{2\ensuremath{\mathrm{i}} } {\bf \a}^\dagger_{x,y+1}\cdot (\sigma_z+\ensuremath{\mathrm{i}}\sigma_x)\cdot {\bf \a}_{x,y} + {\rm h.c.}
\end{align}
The expectation values of these one-body observables can then be read off directly from the elements of the steady-state correlation matrix.

The total particle current flowing, say, into the cold bath is represented by the observable $\hat{J}_{\rm tot} = \ensuremath{\mathrm{i}}[\hat{H}_{\rm tot}, \hat{N}_c]$, where $\hat{N}_c = \sum_{j\in c}\sum_q \hat{b}_{qj}^\dag \hat{b}_{qj}$ is the particle-number operator of the cold bath. Following a similar calculation to Sec.~\ref{app:solution}, we find the standard Landauer formula for the mean steady-state current~\cite{Ryndyk2016}
\begin{equation}\label{J_tot}
J_{\rm tot} = \int\frac{\mathrm{d}	\omega}{2\pi} \,\mathcal{T}(\omega) \left [\bar{n}_h(\omega) - \bar{n}_c(\omega)\right ],
\end{equation}
where $\mathcal{T}(\omega) = \mathrm{Tr}\left [ \mathbf{\Gamma}_c\cdot \mathbf{G} \cdot\mathbf{\Gamma}_h\cdot \mathbf{G}^\dagger\right ]$ is the transmission function. Particle conservation implies that $\sum_y J^X_{x,y} = J_{\rm tot}$ in the NESS.

\subsection{Particle-hole symmetry}
\label{app:PH_symmetry}

In the fermionic setting, the system obeys a generalized particle-hole (GPH) symmetry \cite{Chiu2016} when $\mu=\omega_0$. It is simplest to first analyse this situation assuming that $\omega_0=0$.  In this case,  the fermionic Hamiltonian [Eqs.~(1)--(3)] is invariant under the combined flavor swap and particle hole transformation,  $\hat{\Upsilon}\mathbf{\hat{a}}_{x,y}^\dagger\hat{\Upsilon}^{\dagger} = (\sigma_x \mathbf{\hat{a}}_{x,y})^{\rm T}$ or, explicitly,  $\hat{\Upsilon}(\hat{a}^\dagger_{x,y,\uparrow}, \hat{a}^\dagger_{x,y,\downarrow})\hat{\Upsilon}^{\dagger} = (\hat{a}_{x,y,\downarrow}, \hat{a}_{x,y,\uparrow})$. Meanwhile, the current operators defined in Eqs.~\eqref{current_op_X} and~\eqref{current_op_Y} are odd under this transformation, i.e.~$\hat{\Upsilon}\hat{J}^{X,Y}_{x,y} \hat{\Upsilon}^{\dagger} = -\hat{J}^{X,Y}_{x,y}$. It follows that any state $\hat{\rho}$ that is GPH-invariant, satisfying $[\hat{\rho},\hat{\Upsilon}] = 0$, has vanishing currents. Indeed, schematically we have $\braket{\hat{J}} = \mathrm{Tr}[\hat{J}\hat{\rho}] = -\mathrm{Tr}[\hat{\Upsilon}\hat{J}\hat{\Upsilon}^{\dagger}\hat{\rho}] = -\braket{\hat{J}}$, where $\hat{J}$ stands for any current operator that is GPH-odd.

In general, the correlation matrix can be written in block form as
\begin{equation}\label{C_block}
	\mathbf{C} = \left ( \begin{matrix}
		\mathbf{C}_{\uparrow \uparrow} & \mathbf{C}_{\uparrow \downarrow}\\		\mathbf{C}_{\downarrow \uparrow} & \mathbf{C}_{\downarrow \downarrow}
	\end{matrix}\right ),
\end{equation}
where $\mathbf{C}_{\uparrow \uparrow}$ is the correlation matrix for the $\uparrow$ flavor, $\mathbf{C}_{\uparrow \downarrow} = \mathbf{C}_{\downarrow \uparrow}^\dagger $ describes coherences between the different flavors, etc. The condition for GPH-invariance, $[\hat{\rho},\hat{\Upsilon}] = 0$, implies that the fermionic correlation matrix satisfies
\begin{equation}\label{PH_symmetry_C}
	\mathbf{C} = \mathbf{1} - \mathbf{S}\cdot\mathbf{C}^*\cdot \mathbf{S},
\end{equation}
where $\mathbf{S}$ is a matrix that swaps the flavors, and $\mathbf{C}^*$ is the complex conjugate of $\mathbf{C}$. With the basis order implicit in Eq.~\eqref{C_block}, we have
\begin{equation}\label{S_matrix}
	\mathbf{S} = \left ( \begin{matrix}
		 \mathbf{0} & \mathbf{1}\\	\mathbf{1} & \mathbf{0}
	\end{matrix}\right ),
\end{equation}
where $\mathbf{0}$ is the zero matrix. The GPH symmetry of the many-body Hamiltonian translates to the condition
\begin{equation}\label{PH_single_particle_H}
	\mathbf{H} = -\mathbf{S}\cdot\mathbf{H}^*\cdot\mathbf{S}.
\end{equation}
In turn, this implies the following constraint on the retarded Green function:
\begin{equation}\label{PH_Green_function}
	\mathbf{G}(-\omega) = - \mathbf{S}\cdot\left [\mathbf{G}(\omega)\right ]^*\cdot\mathbf{S}.
\end{equation}
Note that here we assume the self-energy is also GPH-symmetric, i.e.~$\mathbf{\Sigma}(\omega) = -\mathbf{S}\cdot[\mathbf{\Sigma}(-\omega)]^*\cdot\mathbf{S}$. In particular, this applies when the system-bath coupling is identical for both flavor states, so that $[\mathbf{\Sigma},\mathbf{S}] =0$, and when the spectral densities are symmetric, $\gamma_j(\omega) = \gamma_j(-\omega)$.

At the GPH-symmetric point, $\mu=0$, the distribution functions satisfy $\bar{n}_{h,c}(\omega) =  1 - \bar{n}_{h,c}(-\omega)$. Thus, reversing the dummy integration variable as $\omega \to -\omega$ in Eq.~(4), we obtain
\begin{align}
	\label{C_PH_derivation}
\mathbf{C} & = \int\frac{\mathrm{d}\omega}{2\pi} \, \mathbf{G}(\omega) \cdot \Big [\mathbf{ \Gamma}_h \bar{n}_h(\omega) + \mathbf{\Gamma}_c \bar{n}_c(\omega)\Big]\cdot \mathbf{G}^\dagger(\omega)\notag \\
 & = \int\frac{\mathrm{d}\omega}{2\pi} \, \mathbf{G}(\omega) \cdot \Big [\mathbf{ \Gamma} - \mathbf{ \Gamma}_h \bar{n}_h(-\omega) - \mathbf{\Gamma}_c \bar{n}_c(-\omega)\Big]\cdot\mathbf{G}^\dagger(\omega)\notag \\
& =  \mathbf{1} - \int\frac{\mathrm{d}\omega}{2\pi} \, \mathbf{G}(-\omega) \cdot \Big[ \mathbf{ \Gamma}_h \bar{n}_h(\omega) + \mathbf{\Gamma}_c \bar{n}_c(\omega)\Big]\cdot\mathbf{G}^\dagger(-\omega)\notag \\
& =  \mathbf{1} - \mathbf{S}\cdot\mathbf{C}^*\cdot \mathbf{S}.
\end{align}
Above, we have made use of Eq.~\eqref{PH_Green_function} as well as the identity $\mathbf{G}\cdot \mathbf{\Gamma}\cdot \mathbf{G}^\dagger = \ensuremath{\mathrm{i}} \left (\textbf{G} - \mathbf{G}^\dagger\right )$ and the property
\begin{equation}\label{commutation_Gret}
\int\frac{\mathrm{d}\omega}{2\pi }\ensuremath{\mathrm{i}}  \left (\textbf{G} - \mathbf{G}^\dagger \right ) = \mathbf{1},
\end{equation}
which follows from the (anti-)commutation relations~\cite{Kamenev2009}. Since the NESS is the unique Gaussian state with correlation matrix given by Eq.~\eqref{C_PH_derivation}, it follows that the state is GPH-symmetric when $\mu= \omega_0 = 0$. This implies that all currents vanish. Consistent with this observation, GPH symmetry implies that the transmission function is even, $\mathcal{T}(\omega) = \mathcal{T}(-\omega)$, and therefore the integral in Eq.~\eqref{J_tot} is odd and equates to zero.

The same GPH symmetries and associated vanishing currents are obtained when $\mu = \omega_0 \neq 0$. This can be shown simply by shifting the frequency variable $\omega\to \omega +\mu$ in Eq.~\eqref{C_PH_derivation}. The final result then follows from the GPH symmetry of the shifted Hamiltonian $\mathbf{H}' = \mathbf{H}-\omega_0\mathbf{1}$. We have numerically confirmed the GPH symmetry of the NESS in the wide-band limit when $\mu=\omega_0$, both in weak- and strong-coupling regimes.

\subsection{Weak-coupling limit}
\label{app:weak_coupling}

Following Ref.~\cite{Dhar2012}, we show that in the weak-coupling limit the NESS reduces to an energy-diagonal density matrix that coincides with the solution of the secular-Born-Markov master equation~\cite{Breuer2002,RivasHuelga,Rivas2017}. The system Hamiltonian can be written in its spectral representation
\begin{equation}\label{single_particle_H_diag}
	\mathbf{H} = \mathbf{U}\cdot\mathbf{\Omega}\cdot\mathbf{U}^\dagger,
\end{equation}
where $\mathbf{\Omega} = {\rm diag}\{\omega_\alpha\}$ and $\mathbf{U}$ comprise the eigenvalues and eigenvectors of $\mathbf{H}$. The many-body Hamiltonian in this basis reads as
\begin{equation}\label{many_body_H_diag}
\hat{H} = \sum_{\alpha} \omega_\alpha \ensuremath{\hat{c}^\dagger}_\alpha \c_\alpha, \qquad \c_\alpha = \sum_{j} U^*_{j\alpha}\a_j	.
\end{equation}

Now consider the retarded Green function~\eqref{G_ret} in the wide-band limit, $\mathbf{\Sigma} = -\ensuremath{\mathrm{i}} \mathbf{\Gamma}/2 \propto \gamma$. As $\gamma\to 0$, $\mathbf{G}(\omega)$ becomes approximately diagonal in the energy representation. Following identical arguments to Ref.~\cite{Dhar2012}, we obtain the steady-state correlation matrix in the energy eigenbasis as
\begin{equation}\label{diagonal_NESS}
\braket{\ensuremath{\hat{c}^\dagger}_\alpha \c_{\alpha'}} = \delta_{\alpha\alpha'} \frac{s_\alpha \bar{n}_h(\omega_\alpha) + r_\alpha \bar{n}_c(\omega_\alpha)}{s_\alpha + r_\alpha},
\end{equation}
where $s_\alpha$ and $r_\alpha$ describe the dimensionless coupling strength of eigenmode $\alpha$ to the hot and cold baths, respectively:
\begin{align}
\label{s_alpha}
& s_\alpha = \gamma^{-1}\sum_{j,k}U^*_{j\alpha} [\Gamma_h]_{jk}	U_{k\alpha} = \sum_{y=1}^{L_Y}\sum_{\sigma=\uparrow,\downarrow} |U_{(1,y,\sigma),\alpha}|^2,\\
\label{r_alpha}
& r_\alpha = \gamma^{-1}\sum_{j,k}U^*_{j\alpha} [\Gamma_c]_{jk}	U_{k\alpha} = \sum_{y=1}^{L_Y}\sum_{\sigma=\uparrow,\downarrow} |U_{(L_X,y,\sigma),\alpha}|^2.
\end{align}

We now consider the Lindblad master equation obtained within the Born-Markov and secular approximations. Following the standard derivation~\cite{Breuer2002,RivasHuelga} yields the master equation
\begin{equation}\label{Lindblad}
	\dot{\hat{\rho}} = -\ensuremath{\mathrm{i}} [\hat{H}, \hat{\rho}] + \mathcal{L}_h\hat{\rho} + \mathcal{L}_c\hat{\rho},
\end{equation}
with dissipators for the hot and cold baths given respectively by
\begin{align}
	\label{hot_dissipator}
	\mathcal{L}_h = \gamma \sum_\alpha s_\alpha \left ( \bar{n}_h(\omega_\alpha)\mathcal{D}[\ensuremath{\hat{c}^\dagger}_\alpha] + [1\mp \bar{n}_h(\omega_\alpha)]\mathcal{D}[\c_\alpha]  \right ),\\
		\label{cold_dissipator}
	\mathcal{L}_c = \gamma \sum_\alpha r_\alpha \left ( \bar{n}_c(\omega_\alpha)\mathcal{D}[\ensuremath{\hat{c}^\dagger}_\alpha] + [1\mp \bar{n}_c(\omega_\alpha)]\mathcal{D}[\c_\alpha]  \right ),
\end{align}
where $\mathcal{D}[\hat{L}]\bullet  = \hat{L}\bullet \hat{L}^\dagger - \tfrac{1}{2}\{\hat{L}^\dagger \hat{L},\bullet\}$ is a Lindblad superoperator and the plus (minus) sign is for bosons (fermions). It is easy to check that the steady-state solution of Eq.~\eqref{Lindblad}, $\dot{\hat{\rho}}=0$, is a Gaussian state with correlation matrix given exactly by Eq.~\eqref{diagonal_NESS}.

As is well known, the Lindblad equation~\eqref{Lindblad} can be written as
\begin{equation}\label{Lindblad_nonHermitian}
\dot{\hat{\rho}} = -\ensuremath{\mathrm{i}} \hat{H}_{\rm eff} \hat{\rho} + \ensuremath{\mathrm{i}} \hat{\rho} \hat{H}_{\rm eff}^\dagger + \mathcal{J}_h\hat{\rho} + \mathcal{J}_c\hat{\rho},
\end{equation}
where the non-Hermitian Hamiltonian is
\begin{align}\label{H_nonHermitian}
\hat{H}_{\rm eff} & = \hat{H} - \frac{\ensuremath{\mathrm{i}}}{2} \sum_{\alpha} \gamma s_\alpha \left[ \bar{n}_h(\omega_\alpha) + (1\mp 2\bar{n}_{h}(\omega_\alpha)) \hat{c}^\dagger_\alpha \hat{c}_\alpha\right ] \notag \\
& \qquad - \frac{\ensuremath{\mathrm{i}}}{2} \sum_{\alpha} \gamma r_\alpha \left[ \bar{n}_c(\omega_\alpha) + (1\mp 2\bar{n}_{c}(\omega_\alpha)) \hat{c}^\dagger_\alpha \hat{c}_\alpha\right ],
\end{align}
and the superoperators $\mathcal{J}_{c,h}$ represent ``quantum jumps'' due to exchange of particles with the baths~\cite{Plenio1998},
\begin{align}
\label{jump_superoperators}
\mathcal{J}_h\hat{\rho} & = \sum_\alpha \gamma s_\alpha \left [\bar{n}_h(\omega_\alpha) \hat{c}_\alpha^\dagger \hat{\rho}\hat{c}_\alpha + \left (1 + \bar{n}_h(\omega_\alpha)\right ) \hat{c}_\alpha \hat{\rho}\hat{c}_\alpha^\dagger  \right ] ,\\
\mathcal{J}_c\hat{\rho} & = \sum_\alpha \gamma r_\alpha \left [\bar{n}_c(\omega_\alpha) \hat{c}_\alpha^\dagger \hat{\rho}\hat{c}_\alpha + \left (1 + \bar{n}_c(\omega_\alpha)\right ) \hat{c}_\alpha \hat{\rho}\hat{c}_\alpha^\dagger  \right ] .
\end{align}
By including both the non-Hermitian Hamiltonian and the jump terms, we ensure a completely positive and physically consistent description of the full many-body state of the non-equilibrium lattice system, valid at arbitrary times. This is in contrast to non-Hermitian models that neglect the jumps (valid for rare post-selected trajectories of continuously measured systems) or the effective non-Hermitian Hamiltonians appearing in single-particle Green functions, the topological properties of which have recently been of intense interest; e.g., see Ref.~\cite{MartinezAlvarez2018} and references therein.

\begin{figure*}
	\begin{minipage}{0.31\linewidth}
		\includegraphics[width=\linewidth]{impurity_fermion_counter}
	\end{minipage}\quad
	\begin{minipage}{0.31\linewidth}
		\includegraphics[width=\linewidth]{impurity_fermion_highT}
	\end{minipage}\quad
	\begin{minipage}{0.31\linewidth}
		\includegraphics[width=\linewidth]{impurity_fermion_trivial}
	\end{minipage}
	\caption{Current patterns for the same asymmetric impurity distribution shown in Fig.~4(c) but with different parameters. (a,b) Fermionic currents in the topologically nontrivial regime, $m=t$, with on-site energy $\omega_0=10t$, chemical potential $\mu = \omega-0.5t$, and (a) low temperatures, $T_h=t$ and $T_c=0.01t$, or (b) higher temperatures, $T_h=100t$ and $T_c=t$. (c) Same as (a) but showing bosons (red) and fermions (blue) in a topologically trivial regime, $m=3t$. \label{fig:fermion_impurity_quiver}}
\end{figure*}

\subsection{Weak-coupling distribution functions}
\label{app:distribution}

\begin{figure}[b]
	\begin{minipage}{0.495\linewidth}
		\includegraphics[width=\linewidth]{dist_symm}
	\end{minipage}
	\begin{minipage}{0.495\linewidth}
		\includegraphics[width=\linewidth]{dist_asymm}
	\end{minipage}
	\caption{Distribution functions in the NESS for bosons (red) and fermions (blue). (a)~Symmetric impurity configuration shown in Fig.~4(b), with $T_h=t$, $T_c=0.01t$, $\omega_0=10t$ and $\mu=\omega_0-0.1t$. (b)~Asymmetric impurity configuration shown in Fig.~4(c), but with $\mu=\omega_0-0.5t$ as in Fig.~\ref{fig:fermion_impurity_quiver}. Circles show the data for $T_h=t$ and $T_c=0.01t$ [Fig.~\ref{fig:fermion_impurity_quiver}(a)], while light blue squares show the result for fermions at high temperature, $T_h=100t$ and $T_c = t$ [Fig.~\ref{fig:fermion_impurity_quiver}(b)]. The values of $n(\omega_\alpha)$ for bosons are multiplied by $10^3$ to be visible on the same axes. \label{fig:distributions}}
\end{figure}

We now investigate in more detail the form of the weak-coupling distribution function, $n(\omega_\alpha) = \braket{\hat{c}_\alpha^\dagger\hat{c}_\alpha}$, defined by Eq.~\eqref{diagonal_NESS}.  When the reservoirs are at the same temperature, $\bar{n}_h=\bar{n}_c = \bar{n}$, we obtain simply $ n(\omega_\alpha) = \bar{n}(\omega_\alpha)$. This is a smooth, monotonically decreasing function of frequency that is independent of the mode-specific couplings $s_\alpha$ and $r_\alpha$.  As a consequence, the equilibrium currents---as seen, for example, in Fig.~2(c)---are unaffected by the addition of defects in any configuration~\cite{Rivas2017}.

Out of equilibrium, an analogous result is obtained in the clean QWZ model described by Eqs.~(1)--(3) due to the symmetries $\hat{\Pi}\hat{\Theta}\hat{\Sigma}_y$ and $\hat{\Pi}\hat{R}_\pi$. In particular, the symmetry $\hat{\Pi}\hat{\Theta}\hat{\Sigma}_y$ implies that $|U_{(1,y,\sigma),\alpha}|^2 = |U_{(L_X,y,\sigma),\alpha}|^2 $ and therefore $s_\alpha = r_\alpha$ identically. Similarly, the symmetry under $\hat{\Pi}\hat{R}_\pi$ means that $|U_{(1,y,\sigma),\alpha}|^2 = |U_{(L_X,L_Y+1-y,\sigma),\alpha}|^2$, and again $s_\alpha = r_\alpha$ upon summing over $y$ in Eqs.~\eqref{s_alpha} and~\eqref{r_alpha}. As a consequence, the mode occupations~\eqref{diagonal_NESS} become independent of $s_\alpha$ and $r_\alpha$, being given simply by the average of the reservoir distribution functions:
\begin{equation}\label{mode_occ_symmetry}
	n(\omega_\alpha) = \frac{1}{2}\left [\bar{n}_c(\omega_\alpha) + \bar{n}_h(\omega_\alpha) \right ].
\end{equation}
This is again a function of the frequency $\omega_\alpha$ only, and therefore leads to stable current patterns as in the equilibrium case~\cite{Rivas2017}. Any distribution of defects that respects one of the above discrete symmetries will also yield $s_\alpha = r_\alpha$, leading to similar behaviour.

Note that the relevant symmetries are determined both by the Hamiltonian and by the configuration of the baths driving the system out of equilibrium. For example, the transformation $\hat{\Theta}\hat{\Sigma}_x$ is a symmetry of the QWZ Hamiltonian, where $\hat{\Sigma}_x = \hat{R}_{\pi} \hat{\Sigma}_y$ is a reflection about the $x$ axis. However, because this reflection does not interchange the hot and cold baths it is irrelevant for the NESS. Therefore, defect distributions that are only symmetric under $\hat{\Sigma}_x$ destroy the bosonic edge currents whenever $T_c\neq T_h$.

Examples of the nonequilibrium distribution functions obtained for a symmetric defect configuration are shown in Fig.~\ref{fig:distributions}(a), corresponding to the system depicted in Fig.~4(b). As expected, the distributions are well behaved functions of frequency. Conversely, Fig.~\ref{fig:distributions}(b) shows that when the defect configuration does not respect either of the discrete symmetries, as in Figs.~4(c) or~\ref{fig:fermion_impurity_quiver}, the mode occupations are erratically varying functions of frequency. This disrupts the erasure effect and leads to the destruction of the boundary current patterns, in general.

Fig.~\ref{fig:distributions} also shows that the fermionic distributions exhibit a sudden change at the chemical potential whenever $T_c$ is sufficiently small. This sharp feature explains the absence of counter-currents around the impurities in Figs.~4(b,c). In this case, the chemical potential is just below the particle-hole symmetric point $\mu=\omega_0$. This leads to a single ``hole'' that occupies an edge state, visible in Fig.~\ref{fig:distributions} as the isolated point just below $\omega_\alpha=\omega_0$. The edge current pattern observed in Fig.~4(b) is primarily due to this hole state which, occupying an edge mode, is robust against any bulk perturbation. Conversely, when the chemical potential is shifted down to $\mu = \omega_0- 0.5t$, several holes are created in other edge states [Fig.~\ref{fig:distributions}(b), blue circles], including edge states localized around the impurities. Consequently, we see the appearance of counter-currents shielding the impurities in Fig.~\ref{fig:fermion_impurity_quiver}(a).

At higher temperature, the sharp feature in $n(\omega_\alpha)$ disappears [Fig.~\ref{fig:distributions}(b), light blue squares]. The current distribution is then determined mainly by bulk states and thus depends intimately on the symmetries of the impurity configuration. If the configuration is asymmetric, as in Fig.~\ref{fig:fermion_impurity_quiver}(b), the boundary currents are strongly disrupted.

In the topologically trivial regime, there are no edge states and both bosons and fermions behave very similarly with respect to the introduction of defects. In particular, asymmetric impurity distributions tend to inhibit the formation of clean boundary current patterns. An example is shown in Fig.~\ref{fig:fermion_impurity_quiver}(c).

\begin{figure*}
	\includegraphics[width=0.99\linewidth]{semiclassical}
	\caption{The emergence of edge currents in the weak coupling limit can be understood by a semiclassical argument. (a) The factor $n[\omega_-(\mathbf{k})]-n[\omega_+(\mathbf{k})]$ in Eq. \eqref{semi-classical_edge_current} for the bosonic case with $\omega_0=10t$, $T_h=t$, $T_c=0.01t$ and $m=2.1t$. (b) The Berry curvature ${\mathcal{F}\!\!}_-(\mathbf{k})$, which has a balanced positive and negative contributions over B.Z. (the zero value plane is depicted in light blue color) as for  $m>2t$ the model is in a trivial phase and ${\mathcal{F}\!\!}_-(\mathbf{k})$ integrates out to zero. (c) The product $\{n[\omega_-(\mathbf{k})]-n[\omega_+(\mathbf{k})]\}{\mathcal{F}\!\!}_-(\mathbf{k})$, which breaks such a balance, leads to a nonvanishing integral in Eq. \eqref{semi-classical_edge_current}. (d) The semiclassical current pattern generated according \eqref{semi-classical_edge_current} for the potential $V(x,y)=(x/8)^{10}+(y/8)^{10}$.  \label{fig:semiclassical}}
\end{figure*}

\subsection{Semiclassical picture}
\label{app:semiclassical}

The behaviour in the weak coupling can be understood by using a semiclassical picture \cite{Xiao2010,Price2012}.  Under periodic boundary conditions,  the QWZ Hamiltonian can be written in the form
\begin{equation}
\hat{H}=\sum_{\mathbf{k}\in \mathrm{B.Z.}} \mathbf{a}_{\mathbf{k}}^\dagger\cdot \mathbf{H}(\mathbf{k})\cdot \mathbf{a}_{\mathbf{k}},
\end{equation}
with $\mathbf{k}=(k_X,k_Y)$ the quasimomentum and
\begin{equation}
	\label{single-particle-Bloch-H}
\mathbf{H}(\mathbf{k})=\omega_0\mathbf{1}+\mathbf{h}(\mathbf{k})\cdot\bm{\sigma},
\end{equation}
where
\begin{equation}
\mathbf{h}(\mathbf{k})=[t_Y\sin(k_Y),t_X\sin(k_X),m+t_X\cos(k_X)+t_Y\cos(k_Y)].
\end{equation}
Note that we have taken a slightly different Hamiltonian with respect to the original reference \cite{Qi2006}.  The two energy bands of the model are then given by
\begin{equation}
\omega_{\pm}(\mathbf{k})=\omega_0\pm |\mathbf{h}(\mathbf{k})|,
\end{equation}
and for the isotropic case considered throughout this work  ($t_X=t_Y=t>0$),
\begin{equation}
|\mathbf{h}(\mathbf{k})|=t\sqrt{\sin^2(k_X)+\sin^2(k_Y)+[m/t+\cos(k_X)+\cos(k_Y)]^2}.
\end{equation}
The action of a force $\mathbf{F}$ modifies the semiclassical equation for the velocity $\mathbf{v}_\alpha$ of a Bloch wave-packet in the band $\omega_{\alpha}(\mathbf{k})$ (assuming the single-particle Hamiltonian~\eqref{single-particle-Bloch-H} is gapped,  i.e.  $m\neq0,\pm 2t$, and $m$ is small enough to justify the semiclassical approximation) as
\begin{equation}\label{Vsem}
\mathbf{v}_\alpha=\frac{\partial \omega_\alpha(\mathbf{k})}{\partial\mathbf{k}}-\mathbf{F}\times \bm{\mathcal{F}}\!\!_\alpha(\mathbf{k}).
\end{equation}
Here, $\bm{\mathcal{F}}\!\!_\alpha(\mathbf{k})=[0,0,{\mathcal{F}\!\!}_\alpha(\mathbf{k})]$, with ${\mathcal{F}\!\!}_\alpha(\mathbf{k})$ the Berry curvature of the band, which, for a two-band model, can be written in the form
\begin{align}
{\mathcal{F}\!\!}_\pm(\mathbf{k})&=\mp\frac{1}{2}\mathbf{n}(\mathbf{k})\cdot\left[\frac{\partial\mathbf{n}(\mathbf{k})}{\partial k_X}\times \frac{\partial\mathbf{n}(\mathbf{k})}{\partial k_Y}\right],
\end{align}
with $\mathbf{n}(\mathbf{k}):=\mathbf{h}(\mathbf{k})/|\mathbf{h}(\mathbf{k})|$. For the QWZ Hamiltonian we find
\begin{equation}
{\mathcal{F}\!\!}_\pm(\mathbf{k})=\frac{\pm\big[\cos(k_X)+\cos(k_Y)+\tfrac{m}{t}\cos(k_X)\cos(k_Y)\big]}{2\big\{\!\sin^2(k_X)+\sin^2(k_Y)+\big[\tfrac{m}{t}+\cos(k_X)+\cos(k_Y)\big]^2\big\}^\frac32}.
\end{equation}
We can now argue for the presence of an edge circulation under open boundary conditions by introducing a confining potential $V(x,y)$ in the semiclassical equation for $\mathbf{v}_\pm$ \eqref{Vsem}.  Assuming that the potential varies slowly on the scale of the lattice, the energy of the wavepacket in the semi-classical approximation is simply $\omega_\alpha(\mathbf{k}) + V(x,y)$~\cite{Xiao2010}. Moreoever, the potential induces a confining force $\mathbf{F}=-\bm{\nabla}V(x,y)$,  which approximately vanishes in the bulk and becomes very large in the boundary of the confined region,
\begin{align}
	\label{edge-bulk-velocity}
\mathbf{v}_\alpha^\mathrm{(bulk)}\simeq  \frac{\partial \omega_\alpha(\mathbf{k})}{\partial\mathbf{k}}, \quad \mathbf{v}_\alpha^\mathrm{(edge)}\simeq \bm{\nabla}V(x,y)\times \bm{\mathcal{F}}\!\!_\alpha(\mathbf{k}).
\end{align}
Since $\mathbf{F}$ is normal and points inward from the confined boundary,  a circulating current is induced along this boundary with direction given the sign of the Berry curvature, which depends on the band $\alpha$, the sign of $m$, and the specific value of $\mathbf{k}$: clockwise for ${\mathcal{F}\!\!}_\alpha(\mathbf{k})>0$ and counterclockwise for ${\mathcal{F}\!\!}_\alpha(\mathbf{k})<0$. Thus, for the NESS at the weak coupling regime,  we may estimate the current density (current per unit width) by \cite{Xiao2010}
\begin{align}
	\label{semiclassical_current}
\mathbf{I}(x,y)=\sum_{\alpha=\pm}\int_{\mathrm{B.Z.}}d^2\mathbf{k}\, n[\omega_\alpha(\mathbf{k})+V(x,y)] \mathbf{v}_\alpha(x,y,\mathbf{k}),
\end{align}
where the integral extends over the first Brillouin zone. Here we have assumed that the NESS occupation number $n$ only depends on energy. As discussed in Sec.~\ref{app:distribution}, this is the case under a $\hat{\Pi}\hat{\Theta}\hat{\Sigma}_y$ or a $\hat{\Pi}\hat{R}_\pi$ symmetric configuration.

Now, if we consider regions far from the boundary, so that $V(x,y)\ll \omega_\alpha(\mathbf{k})$, we may approximate Eq.~\eqref{semiclassical_current} by
\begin{align}
	\mathbf{I}(x,y)&\simeq\int_{\mathrm{B.Z.}}d^2\mathbf{k}\, \{n[\omega_-(\mathbf{k})]-n[\omega_+(\mathbf{k})]\} \mathbf{v}_-,
\end{align}
using the fact that $\mathbf{v}_+= -\mathbf{v}_-$. Since there is no privileged direction of $\mathbf{v}_-^{\mathrm{(bulk)}}$ on each energy shell: $\omega_\alpha(\mathbf{k})=\omega_\alpha(-\mathbf{k})$ and hence $\frac{\partial \omega_\alpha(\mathbf{k})}{\partial\mathbf{k}}=-\frac{\partial \omega_\alpha(-\mathbf{k})}{\partial\mathbf{k}}$. Therefore, the contribution of $\mathbf{v}_\alpha^{(\rm bulk)}$ to the integrand is odd and integrates to zero. We conclude that
\begin{align}
	\label{semi-classical_edge_current}
	\mathbf{I}(x,y)&\simeq\int_{\mathrm{B.Z.}}d^2\mathbf{k}\, \left \{n[\omega_-(\mathbf{k})]-n[\omega_+(\mathbf{k})]\right \} \mathbf{v}_-^{(\rm edge)},
\end{align}
which clearly vanishes in the bulk of the system where $V(x,y)=0$ (see Eq.~\eqref{edge-bulk-velocity}).  Nevertheless, since $n(\omega)$ is a monotonically decreasing function of energy [Eq.~\eqref{mode_occ_symmetry}], there is an imbalance of the contributions to $\mathbf{I}(x,y)$ within the Brillouin zone in regions where $\mathbf{v}_\alpha^{\rm edge} \propto \nabla V(x,y) \neq 0$. Thus, Eq.~\eqref{semi-classical_edge_current} predicts a net chiral edge current,  see Fig. \ref{fig:semiclassical}. This erasure effect sustains the appearance of the chiral current in the symmetric situation, but it is spoilt in the nonsymmetric case,  as the occupation number is no longer only a function of the energy alone.

\section{Results}

	\begin{figure*}
		\begin{minipage}{0.31\linewidth}
			\includegraphics[width=\linewidth]{quiver_strong_combi}
		\end{minipage}\quad
		\begin{minipage}{0.31\linewidth}
			\includegraphics[width=\linewidth]{quiver_weak_combi}
		\end{minipage}\quad
		\begin{minipage}{0.31\linewidth}
			\includegraphics[width=\linewidth]{quiver_eq_combi}
		\end{minipage}
		\caption{Current distributions on a lattice of size $L = 8$. Red arrows show boson currents in a topologically trivial phase ($m=3t$), blue arrows show fermion currents in a topologically nontrivial regime ($m=t$). Arrow sizes indicate the magnitude of the currents scaled relative to the largest value within each plot. (a,b) Nonequilibrium current profile with different temperatures $T_h =  t$ and $T_c= 0.01t$, on-site energy $\omega_0=10t$, chemical potential $\mu = \omega_0-0.01t$ for fermions (we always set $\mu=0$ for bosons), and coupling strength (a)~$\gamma = 0.5t$ and (b)~$ \gamma = 0.005t$. (c)~Equilibrium case with temperatures $T_c=T_h=t$, weak coupling, $\gamma = 0.005t$, and other parameters identical to (a,b). \label{fig:quiver_coupling}}
	\end{figure*}

	\noindent {\em Results.---}In the following examples, we focus on the symmetric case with $L_X = L_Y = L$ and $t_X = t_Y=t$, so that $|m|<2t$ defines the topologically non-trivial phase. We also fix $\omega_0=10t$ and consider relatively low temperatures, $T_{c,h}\lesssim t$, to accentuate the role of band topology and particle exchange statistics.

	\begin{figure}[b]
		\begin{minipage}{0.495\linewidth}
			\includegraphics[width=\linewidth]{edge_bulk_currents_bosons}
		\end{minipage}
		\begin{minipage}{0.495\linewidth}
			\includegraphics[width=\linewidth]{edge_bulk_currents_fermions}
		\end{minipage}
		\caption{Average edge currents, $J_{\rm edge}$ (solid lines), and bulk currents, $J_{\rm bulk}$ (dashed lines), as a function of the system-bath coupling strength, $\gamma$, for bosons (left panel) and fermions (right panel) in topologically non-trivial ($m/t=1$) and trivial ($m/t=2.1,3$) regimes, and with $T_h= t$, $T_c=0.01t$, $\omega_0=10t$, and $\mu = \omega_0+0.1t$. \label{fig:edge_bulk_currents}}
	\end{figure}

	Figs.~\ref{fig:quiver_coupling}(a,b) plot the nonequilibrium current distributions for two different values of the system-reservoir coupling, $\gamma$. Red arrows show the currents for a bosonic system with $m=3t$ (similar results are obtained for $|m|<2t$). Remarkably, the currents become progressively localized on the boundary of the system as $\gamma$ is reduced, even though the band topology is trivial. These edge currents also arise in the equilibrium case, $T_h=T_c$, as shown in Fig.~\ref{fig:quiver_coupling}(c). Qualitatively similar results are obtained for fermions, as shown for a nontrivial phase ($m=t$) by the blue arrows in Fig.~\ref{fig:quiver_coupling}. The direction of fermionic particle flow depends on the chemical potential; for the parameters in Figs.~\ref{fig:quiver_coupling}(a,b), the thermoelectric induced current flows in the opposite direction to the temperature gradient. Conversely, when $\mu=\omega_0$, all currents vanish due to particle-hole symmetry~\cite{SM}.

	In order to quantify the emergence of boundary currents more precisely, we define the average edge and bulk currents
	\begin{align}\label{edge_and_bulk_current}
		J_{\rm edge} &= \frac{1}{2L_X}\sum_{x} \left( J^{X}_{x,L_Y} - J^X_{x,1} \right ), 	\qquad J_{\rm bulk} = \frac{1}{L_Y}\sum_{y} J^{X}_{x,y}.
	\end{align}
	The choice of $x$-coordinate in the definition of $J_{\rm bulk}$ is arbitrary due to particle-number conservation; we take $x=\lfloor L_X/2\rfloor$. The total current flowing between the two reservoirs is given by $J_{\rm tot} = L_Y J_{\rm bulk}$.

	We plot the edge and bulk currents in Fig.~\ref{fig:edge_bulk_currents} for bosonic and fermionic systems as a function of the system-reservoir coupling strength, $\gamma$. In the bosonic case, both bulk and edge currents increase with $m$ and are thus larger in the topologically trivial phase. The situation is reversed for fermions, with the largest edge currents obtained in the topologically nontrivial phase. In all cases, the bulk currents are proportional to $\gamma$ and thus vanish as $\gamma\to 0$, while the edge currents remains invariant for a wide range of values of $\gamma$ and persist in the weak-coupling limit. These quantitative results therefore confirm the qualitative picture of Fig.~\ref{fig:quiver_coupling}, i.e., edge currents arise for small coupling irrespectively of band topology or particle statistics. In topologically trivial phases, edge currents begin to dominate once $\gamma$ becomes comparable to the level spacing of the single-particle Hamiltonian. However, in the topologically nontrivial phase for fermions near half filling,  currents remain localized on the edges even for strong coupling, $\gamma\sim  t$.

	\begin{figure*}
		\begin{minipage}{0.31\linewidth}
			\includegraphics[width=\linewidth]{impurity_edge}
		\end{minipage}\quad
		\begin{minipage}{0.31\linewidth}
			\includegraphics[width=\linewidth]{impurity_sym}
		\end{minipage} \quad
		\begin{minipage}{0.31\linewidth}
			\includegraphics[width=\linewidth]{impurity_asym}
		\end{minipage}
		\caption{Effect of impurities on the current distribution in the weak-coupling limit, with impurity positions marked by filled black circles. Red arrows show boson currents and blue arrows show fermion currents. In all plots, $m=t$, $T_h= t$, $T_c=0.01t$, $\omega_0=10t$ and $\mu = \omega_0 - 0.1t$.\label{fig:quiver_impurities}}
	\end{figure*}

	Finally, we investigate whether these effects withstand the presence of imperfections, a property which defines the notion of dissipatively robust currents. Specifically, we examine how the currents change when static impurities are added to the lattice. Impurities are modelled by a large on-site energy shift, i.e.,~a term $\Delta {\bf\a}^\dagger_{x,y}
	\cdot {\bf \a}_{x,y}$ added to the Hamitonian, where $\Delta \gg \omega_0, t$ and $(x,y)$ are the coordinates of the impurity site~\cite{Rivas2017}. We focus hereafter on the weak-coupling limit where the edge currents are most prominent in the absence of impurities. In this limit, an analytical expression for the NESS~\cite{Dhar2012} can be obtained, which is identical to the solution of the Lindblad equation derived under the Born-Markov and secular approximations~\cite{SM}.

	In Fig.~\ref{fig:quiver_impurities} we show three examples of how impurities affect the nonequilibrium current distribution in the topologically nontrivial phase. We observe substantial differences between bosonic and fermionic systems when one of the reservoirs is at low temperature. The bosonic edge currents are preserved only when the impurity distribution is invariant under one of the symmetries~$\hat{\Pi}\hat{\Theta}\hat{\Sigma}_y$ or $\hat{\Pi}\hat{R}_\pi$, which correspond to the purely spatial symmetries $\hat{\Sigma}_y$ and $\hat{R}_\pi$ since the defects satisfy $\hat{\Pi}$ and $\hat{\Theta}$ automatically. In the case of impurities placed on the edge (and assuming the symmetries are respected in the bosonic case), the currents simply detour around the impurity sites [Fig.~\ref{fig:quiver_impurities}(a)]. If impurities are placed in the bulk of a bosonic system in an appropriately symmetric way, counter-currents shield the impurity sites by circulating in the opposite direction to the edge currents~[Fig.~\ref{fig:quiver_impurities}(b)]. In the absence of these symmetries, the bosonic edge currents are strongly disrupted [Fig.~\ref{fig:quiver_impurities}(c)]. For fermions in a topological phase, the situation is starkly different when at least one reservoir is at low temperature: impurities placed in the bulk have no effect whatsoever on the current distribution~[Figs.~\ref{fig:quiver_impurities}(b,c)]. In the topologically trivial phase or at high temperature, both bosonic and fermionic edge currents enjoy the same symmetry-protected robustness as  bosons in the nontrivial phase.

\noindent {\em Discussion.---}The question posed in the introduction on the nontopological origin of the edge currents can now be answered. In the weak-coupling limit, nonequilibrium coherences between energy eigenstates become small~\cite{Dhar2012} and $J_{\rm bulk}$, which is directly proportional to these coherences~\cite{Mitchison2018}, is negligible in comparison to the contributions from individual energy eigenstates. Moreover, the single-particle eigenmodes in the QWZ model present a nonzero Berry curvature $\bm{\mathcal{F}}_\alpha$ for $m\neq 0$~\cite{Qi2006}, which breaks time-reversal symmetry and endows the eigenmodes with a particular chirality. This can be understood in a semi-classical picture~\cite{Haldane2004}, where a wavepacket propagates with velocity $\mathbf{v}_\alpha = \partial_{\mathbf{k}} \omega_\alpha +  \nabla V \times \bm{\mathcal{F}}_\alpha$, with $\mathbf{k}$ the wavevector and $V(x,y)$ a confining potential describing the edge of the system~\cite{Xiao2010}. Assuming that the non-equilibrium distribution function only depends on energy, the net current due to the derivative term $\partial_{\mathbf{k}} \omega_\alpha$ can be shown to vanish in the bulk due to cancellations between positive and negative wavevectors~\cite{SM}. However, the contribution of the axial force $\nabla V \times \bm{\mathcal{F}}_\alpha$ is non-zero near the boundary, thus generating a net chiral edge current~\cite{SM}. This erasure effect arises whenever there is broken time-reversal symmetry and a smooth, energetically monotonic distribution of chiral eigenmodes~\cite{Rivas2017}; it is thus independent of exchange statistics or band topology. Intuitively, the effect can be understood in terms of circulating currents that cancel in the bulk but add constructively on the boundary [Fig.~\ref{fig:QWZ}(b)].

A chiral current between two thermal reservoirs unavoidably entails a local cross-current phenomenon:  on one edge there are particles flowing from the cold bath to the hot bath. In bosonic systems, this implies a ``violation'' of the second law of thermodynamics within a one-dimensional subsystem, i.e.,~energy flows against the temperature gradient along one edge even though the total rate of entropy production is positive. This effect was reported in Refs.~\cite{Rivas2017,Xing2020} for bosonic lattices governed by the Hofstadter Hamiltonian. Now, we see that the key requisite for this behavior is not the nontrivial band topology of the lattice, but rather the nonzero Berry curvature in a regime of weak system-bath coupling [Fig.~\ref{fig:quiver_coupling}(b,c)].

The edge currents are robust to impurities if the defect distribution satisfies either of the symmetries $\hat{\Pi}\hat{\Theta}\hat{\Sigma}_y$ or $\hat{\Pi}\hat{R}_\pi$. Note that the relevant nonequilibrium symmetries are determined both by the Hamiltonian and by the configuration of the baths. These symmetries leave the NESS invariant and lead to a steady-state correlation matrix that is independent of the spatial orientation of the reservoirs. Under these conditions, the nonequilibrium distribution function is simply the average of the reservoir distributions~\cite{SM}, i.e.,~$n(\omega_\alpha) = \tfrac{1}{2}\left [ \bar{n}_h(\omega_\alpha) + \bar{n}_c(\omega_\alpha)\right ]$ is the population of the eigenmode with frequency $\omega_\alpha$. This smooth distribution function yields boundary currents due to the erasure effect in the bulk. In the absence of symmetry, however, the contribution of each mode depends not only on energy but also on the spatial profile of the corresponding wavefunction. This creates an erratically varying distribution function that destroys the erasure effect~\cite{SM}.

For fermions at low temperature $T_c$, $n(\omega_\alpha$) undergoes a sharp change near $\omega_\alpha \approx \mu$. In a topologically nontrivial phase near half filling, this feature acts as a filter that populates only one or two edge states~\cite{SM}, which are topologically protected against perturbations in the bulk. The corresponding boundary current is thus completely unaffected by impurities [Figs.~\ref{fig:quiver_impurities}(b,c)]. Remarkably, this holds for arbitrarily large $T_h$, providing an instance of a topologically protected property that is also stable under dissipation. The number and character of edge modes that contribute to the current pattern is determined by the chemical potential~\cite{SM}.

In summary, our nonperturbative analysis has shown that robust boundary currents emerge at weak coupling in the QWZ lattice driven out of equilibrium by a thermal gradient. Our results reveal a novel dissipative mechanism for symmetry-protected edge transport, which arises in bosonic and fermionic systems with and without nontrivial band topology. This makes quantum simulators based on either fermionic or bosonic degrees of freedom attractive candidates to observe this exotic boundary physics.

\textit{Acknowledgements.---}M.~T.~M. acknowledges funding from the ERC Starting  Grant ODYSSEY (Grant  Agreement No.~758403) and the EPSRC-SFI Joint Funding of Research project QuamNESS. A.~R. and M.~A.~M.-D. acknowledge financial support from the Spanish MINECO grants MINECO/FEDER Projects FIS2017-91460-EXP, PGC2018-099169-B-I00 FIS-2018 and from CAM/FEDER Project No. S2018/TCS-4342 (QUITEMAD-CM). The research of A.~R. and M.~A.~M.-D. has been partially supported by the U.S. Army Research Office through Grant No.~W911NF-14-1-0103. Calculations were performed on the Lonsdale cluster maintained by the Trinity Centre for High Performance Computing. This cluster was funded through grants from SFI.

	\bibliographystyle{apsrev4-2}

redpajama_set_name: RedPajamaArXiv


text:
Notebook: Daniel Jones ruled out vs. Chargers; Mike Glennon clears concussion protocol
Michael Eisen
Giants.com Senior Writer/Editor
TUCSON, Ariz. – Quarterback Daniel Jones was one of three players officially declared out of the game Sunday in Los Angeles against the Chargers. He will be inactive for a second straight week because of the neck injury he suffered against Philadelphia on Nov. 28.
Mike Glennon will start for Jones, as he did last week in Miami. Glennon cleared the NFL concussion protocol on Friday afternoon.
Wide receiver Kadarius Toney (oblique) and cornerback Adoree' Jackson (quad) will also not play. Toney will miss his third consecutive game and fourth of the season and Jackson will be inactive for the second week in a row.
Defensive lineman Danny Shelton did not practice and was added to the injury report as questionable with a calf injury. Wide receivers Kenny Golladay (rib) and Sterling Shepard (quad) are also questionable.
*Coach Joe Judge wore an Arizona hoodie and cap to practice today. For three days, the Giants used the Wildcats' facilities and practice field to prepare for Sunday's game. Judge said the week here was a big success.
"It's been a good, productive week for us so far," Judge said. "It's been very good for the team being out here. I'm very appreciative of the University of Arizona extending the facilities, what they've offered and worked with us on. Couldn't be more grateful. I know they're very busy themselves right now, they're in the middle of a big recruiting weekend, so the staff themselves are all back in off the road. There's a lot of gymnastics going on in the building, but they've completely let us have free run of whatever we want, whatever we need. Couldn't be more appreciative of that."
Some players were skeptical about spending a week away from home, but those sentiments seemed to have evaporated in the desert. Two of the team's captains gave the trip high marks.
"It's a refresh," running back Saquon Barkley said. "Just being in a different state, different weather. I like it because it's kind of like college. You're forced to be with your teammates a lot more. When you go home after practice, usually you go home – I go home to my family. (Tight end Kyle) Rudolph goes home to his family. (Tackle Nate) Solder goes home to his family. It's a different environment when you're home. When you're here, (it's) not a bad thing, meaning being forced, but we're put in hotels. We're eating together more. We're talking crap, playing games, watching football together – all the stuff that you kind of have in college ball and you miss. You don't really have that when you get to the NFL. That's why I think it's beneficial for the team also, too."
"I think it was good to get away, reset our minds a little bit," safety Logan Ryan said. "We had a really spirited practice (yesterday) – two hours in the pads getting after it, having some of their (Arizona's) team out here watching us play at the highest level and having some kids warm up with us. It's really cool, there are Giants fans all over the place. We've got a great fan base. But it's been a really good week. Kind of training camp mentality of just hanging out in the hotel room, watching film, going to the basketball game together, going to dinners together. It's been really good just to get around the guys and support our guys."
*Linebacker Blake Martinez spoke publicly for the first time since tearing his ACL on Sept. 26 against Atlanta. He underwent surgery and is rehabbing his knee.
Martinez is a Tucson native but did not play at the state – and local - university.
"I have my bittersweet moments here – they didn't want me to play here, so went to Stanford and became smart," Martinez said with a smile. "But no, it's good. I've been kind of the tour guide showing people around, showing them good spots to eat and things like that."
Martinez said his rehab is going well.
"I'm feeling good," he said. "Just kind of working out every day, trying to stay consistent, working with the training staff and strength staff, making sure I make improvements. Keep working through it.
"Right now, it's just progressing. There are certain checkpoints and things like that, but as you can see, I'm able to start walking. Things like moving, bodyweight work in the training room, nothing heavy or anything. It's been good to finally – mentally for me – to be able to do stuff like that again."
New York Giants vs. Los Angeles Chargers: How to Watch, Listen & Live Stream Week 14
📸 Practice Photos: Giants train in Arizona
View photos from practice at the University of Arizona as the Giants prepare for their matchup against the Chargers.
Saquon Barkley (26)
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redpajama_set_name: RedPajamaCommonCrawl


That it takes years to build up trust, and only … seconds to destroy it. That it's not what you have in your life but who you have in your life that counts.
That you can get by on charm for about fifteen minutes. After that, you better know something. That you shouldn't compare yourself to the best others can do. That you can do something in an instant that will give you heartache for life.
That it's taking me a long time to become the person that I want to be. That you should always leave loved ones with loving words. It may be the last time you see them.
That you can keep going long after you can't. That we are responsible for what we do, no matter how we feel.
That either you control your attitude or it controls you. That regardless of how hot and steamy a relationship is a first, the passion fades and there had better be something else to take its place.
That heroes are the people who do what has to be done when it needs to be done, regardless of the consequences. That money is a lousy way of keeping score.
That my best friend and I can do anything or nothing and have the best time. That sometimes the people you expect to kick you when you are down will be the ones to help you get back up.
That sometimes when I get angry I have the right to be angry, but it doesn't give me the right to be cruel. That true friendship continues to grow over the longest distance, and the same goes for true love.
That just because someone doesn't love you the way you want them to doesn't mean they don't love you with all they have. That maturity has more to do with what types of experiences you've had and what you've learned from them and less to do with how many birthdays you've celebrated.
That you should never tell a child their dreams are unlikely or outlandish. Few things are more humiliating, and what tragedy it would be if they believed it. That no matter how good your friend is, they're going to hurt you every once in a while, and you must forgive them for that.
That it isn't always good enough to be forgiven by others. Sometimes you must learn to forgive yourself. That no matter how bad a heart is broken; the world doesn't stop for your grief.
That our background and circumstances may have influenced who we are, but we are responsible for whom we become. That just because two people argue, it doesn't mean that they don't love each other, and just because they don't argue, it doesn't mean they do.
That we don't have to change friends, if we understand that friends change. That two people can look at the exact same thing and see something totally different.
That your life can be changed in a matter of hours by people who don't even know you. That even when you think you have no more to give, when a friend cries out to you, you will find the strength to help.
That it ¡s hard to determine where to draw the line between being nice and not hurting someone's feelings or standing up for what you believe. That no matter what happens to me on earth or how much my faith falters, God's faith in me never dwindles or fails.
That life's lessons never end and wisdom can always be passed on.


Title - "Everything because he was hungry"
They wanted to translate what he is saying so they needed a translator.
- Does someone know where are the Gheists.
- I know only they are under ground.
William found traces from Anibal so they will lead to the Gheists.
- I will help you if you give me slime and white rat DNA.
- Now we need only white rat DNA.
William spitted a white rat.
- Vryer, we are ready.
- So fast. OK what do you need?
- A translator machine. For a Ghumbo creature.
- Here you are : GT4300.
- Thank you know let's translate.
- Aaaa. Where is Ghumbo.
- We forgot him on the road. Fast.
Where is Mammamara. Huna akatearau.
- Put the translator on level Ghumbo. Not Werewolf.
Where am I? Who are these guys? Here I can't find other like me. I can't find good food too.
Hey strange looking people. Is there any food with you.
I want fish. I ate one golden, one grey and one which was 2D. And when I ate them – my mouth begins bleeding and releases my poison slime.
She came in the same moment.
- Yes. Thank you, you found him. Hello Ghumbo. I will help you. Come with me.
Ghumbo touched her and they disappeared.
I saw that on the message board some sentences disappeared. The chapters weren't more than 1500. I don't know why that happened.


text:
Artmap
ZKM | Zentrum für Kunst und Medientechnologie
fast forward 2. The Power of Motion | Media Art Sammlung Goetz
18 Jun - 03 Oct 2010
Janine Antoni »Touch«, 2002, Filmstill, Courtesy Sammlung Goetz, © Janine Antoni
ZKM | Museum of Contemporary Art
Seven years after "fast forward," the exhibition "fast forward 2" will show a wide range of new video acquisitions from the internationally renowned private collection of Ingvild Goetz from Munich. With her impressive collection, originating from the 1960s, she has put together a museum-quality panorama of contemporary art that is as comprehensive as it is personal. Ingvild Goetz was one of the few private collectors to become involved in video art early on, and consistently. She led the way with this position, as video art deals with technically complex works that are often very costly to care for and install. Over the years, Ingvild Goetz has been able to build up a media art collection that is internationally regarded as one of the most important in the world.
In order to do justice to the collection, the museum building built in 1993 by Herzog/de Meuron in Munich was expanded with BASE103 in 2004. The exhibitions in the collection are a plea for an openness of perception and a steady readjusting of thoughts and notions.
ZKM offers for the second time, the opportunity to see a representative selection of media works from the collection: presented will be roughly 60 videos, video installations, and films from thirty artists. Focus of the exhibited works is current productions from 2000 to today. It is the collector's personal concern to show also works by the "youngest generation."
Video-based works are already firmly established as a means of expression in our era. The development of generally valid social questions from personal perspectives is the starting point of many works in this collection.
A great number of artists represented in the Sammlung Goetz do not produce their works for the "white cube" of the museum, but rather, for the cinema. For this reason, the exhibition will be accompanied by a film program shown in the media theater.
An extensive catalogue of works will be published for the exhibition.
Curators: Ingvild Goetz and Stephan Urbaschek
Artists (preliminary list): Francis Alys, Matthew Barney, Janet Cardif/Georges Bures Miller, Christoph Brech, Paul Chan, Keren Cytter, Nathalie Djurberg, Juan Manuel Echavarria, Omer Fast, Rodney Graham, Agneta Grzeszykowska, Johan Grimonprez (Kino), Sven Johne, Isaac Julien, Mike Kelley, Jochen Kuhn (Kino), Tim Lee, Ulrike Ottinger (Kino), Paul Pfeiffer, Robin Rhode, Pipilotti Rist (Kino), Julian Rosefeldt, Wilhelm Sasnal, Christine Schulz, Kelley Walker, Artur Zmijewski
www.zkm.de
Tags: Francis Alÿs, Matthew Barney, Christoph Brech, Paul Chan, Keren Cytter, Nathalie Djurberg, Juan Manuel Echavarría, Omer Fast, Rodney Graham, Johan Grimonprez, Sven Johne, Isaac Julien, Mike Kelley, Tim Lee, Herzog & De Meuron, Ulrike Ottinger, Paul Pfeiffer, Robin Rhode, Pipilotti Rist, Julian Rosefeldt, Wilhelm Sasnal, Kelley Walker, Artur Zmijewski
Edit ZKM | Zentrum für Kunst und Medientechnologie
Theo Jansen
Bundeskunsthalle
Bani Abidi
Gropius Bau
Witte de With
Stedelijk Museum
n.b.k.
HangarBicocca
Ruhr Ding: Territories
Urbane Künste Ruhr
Hysterical Mining
Kunsthalle Wien
Tate Britain
Kunsthalle Basel
58. Biennale di Venezia
33. São Paulo Biennial
6. Athens Biennale
Riga Biennial 2018
Liverpool Biennial 2018
Steirischer Herbst 2018
10th Berlin Biennale 2018
Made in L.A. 2018
Biennale of Sydney 2018
New Museum Triennial
Skulptur Projekte Münster
Documenta 14 Kassel
Documenta 14 Athens
Manifesta 11 Zürich
© Artmap Foundation


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text:
COLORADO ADOPTION SEARCH AND REUNION
PLEASE CHECK THE FREQUENTLY ASKED QUESTIONS PAGE
PAGE LAST UPDATED 7/2/2018
© 1996 to 2018, in honor of Rema/Ellen.
This website may be freely linked but not reproduced or redistributed.
SUBMIT A LINK, MAKE A SUGGESTION,
TELL US ABOUT A NEW RESOURCE
OR LEAVE A COMMENT:
ORPHANAGES AND HOMES
AFFILIATEDCHILDREN'S FAMILY SERVICES INC
For African American children in 1977. Appears that though they started some adoptions none were ever completed. No records.
AMERICAN LEGION CHILD WELFARE
Under the auspices of the American Legion. Residential care of children. No records available. Headquarters is in Indianapolis IN.
CLAYTON HOME FOR BOYS
Care for boys 6 to 18 years. 1911. No known adoptions or records.
COLORADO CHILDREN'S AID SOCIETY
Records may be at Human Services.
COLORADO CHRISTIAN HOME
Established as part of the 'Orphan Trains'. Primarily an orphanage but did do some adoptions. Records can be found at Tennyson Center 4325 W. 29th Av Denver CO 80212. Sharon Carr 303-433-8002
DENVER CHILDREN'S HOME
Part of the 'Orphans Train' now a residential treatment center. Richard Wong 303-399-4890
HOUSE OF THE GOOD SHEPHERD
For problem and delinquent girls operated by the Catholic Sisters of the Good Shepherd. Records may be at the Department of Institutions. Can also check with the Archdiocese of Denver.
INFANT OF PRAGUE ORPHANAGE
Orphanage opened in March 1946 as the Deanery Nursery Home, run by the Sisters of St. Francis. Started in the building that was at one time called the St. Clara's Orphanage. It moved numerous times in the early days. The Orphanage was closed in 1972. They did their own adoptions through about 1954. Adoptions in later years were done through Catholic Charities and they now hold most of the records for the Orphanage. Check with the Denver Catholic Archdiocese for records.
J. K. MULLEN HOME FOR BOYS
Catholic day school run by the Christian Brothers of the Catholic Church and residential care for orphan boys. For possible records try the Little Sisters of the Poor 3629 W 29th Av Denver CO
Phone: 303-761-1764. Records ext. 3307 or alumni office ext. 3336
MCDONALD'S MATERNITY HOSPITAL
1925 through at least 1947. No records found.
MOUNT ST VINCENT HOME
Orphanage began with the 'Orphan Trains'. Originally called the St Vincent's Orphan Asylum started by the Catholic Sisters of Charity of Leavenworth KS. Early records were burned in a fire that destroyed the building in 1902. 1969 to present, now a treatment center for children suffering from trauma. https://www.msvhome.org/
QUEEN OF HEAVEN ORPHANAGE
1902 to 1970 Catholic home for orphan girls. Mother Cabrini Memorial School run by the Missionary Sisters of the Sacred Heart. No records of adoptions, no records found. See below.
SAINT CLARA ORPHANAGE
Run by the Franciscan Sisters, Daughters of the Sacred Hearts of Jesus & Mary. No records of adoptions.
Sacramental records for Saint Clara's and Queen of Heaven are held in the Archdiocese Archives.
https://archden.org/archives/
Karyl Klein
Karyl.Klein@archden.org
STATE: FORMERLY COLORADO DEPARTMENT OF SOCIAL SERVICES, FAMILY AND CHILDRENS WELFARE, PUBLIC WELFARE, CHILD WELFARE...
Now called The Department of Human Services. Seems to have gone through several name changes with the progression of lawmakers. Note: The State did not do any adoptions, but they now hold the records of all the adoptions that were handled through the counties in Colorado.
For adoptees who were in the custody of a county human service agency before adoption:
Colorado Department of Human Services
Adoption Unit
1575 Sherman St., Second Floor
STATE HOME FOR DEPENDENT & NEGLECTED CHILDREN
Established in 1895. Once called Colorado State Children's Home, and then Colorado Youth Center. These records were held at the Colorado State Home, Adoption Records Division of Youth Services, but they have now been transferred to the State of Colorado, Department of Human Services, Adoption Services Unit. Michelle Lopez can be reached by calling 303- 866-3209, or by emailing michelle.lopez2@state.co.us. She has records on the adoption of children that were a ward of the State Home for Dependent and Neglected Children prior to being adopted. If you do not know if you were a ward of the state, then you can call her, and she will check for your records. She has records dating from March 1896 to July 1971.
HOLY FAMILY ORPHANAGE
Catholic orphanage run by the Capuchin Sisters. Records can be found at the Western Research Library in Pueblo. Robert Collyer has done a great deal of work in finding these old records. He also has records for McClelland Orphanage. To contact him call (719) 543-7211 or write to him, 7A Windbridge Lane, Pueblo, CO 81001
LINCOLN HOME
A private institution for African American children established in 1905. No known adoptions.
2723 North Grand, Pueblo CO 81003
MCCLELLAND ORPHANAGE FOUNDATION
In operation in the early part of this century through at least 1930. It is now called the McClelland School. I have been told that some records for McClelland Orphanage can be found at the Western Research Library in Pueblo. Robert Collyer has done a great deal of work in finding these old records. To contact him call (719) 543-7211 or write to him, 7A Windbridge Lane, Pueblo, CO 81001
SACRED HEART ORPHANAGE
Catholic home for emotionally disturbed teens. Might check with the Archdiocese.
BELLEVIEW SCHOOL
WESTMINSTER SCHOOL
Run by the Pillar of Fire Church. No records
WESTMINSTER SHELTER CARE
Division of Human Services. 7640 Lowell Blvd Westminster CO 80030


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text:
In Wisconsin, Shades of the Thirties
by Dick Meister
By now, there's can be no doubting it: What's happening in Wisconsin is one of the most important labor developments in decades. It's of major importance to unions and their members, of major importance to working people generally  of major importance to us all.
In many ways, it's the 1930s again. Just as then, workers and their political allies and other supporters are demonstrating, picketing, marching, striking and otherwise forcefully demanding the basic civil right of collective bargaining  the unfettered right for workers' representatives to negotiate with employers on setting their wages, hours and working conditions.
Eventually, workers and their millions of supporters won the 1930s struggle.
Congress, acting closely with President Franklin D. Roosevelt, granted the legal right of collective bargaining to most workers. Farm workers, domestics and a few other groups were excluded from the law, but all others finally had that vital right.
The 1930s struggle arose primarily because of the economic pressures of the Great Depression that led to massive protests, just as today's struggle can be traced to the pressures of the Great Recession that also have led to massive protests.
There are key differences between then and now, however. In the thirties, the struggle was to win union rights for workers in the face of strong opposition from large financial interests, powerful conservative politicians and other anti-labor forces. Today, the struggle is to keep union rights from being taken away from workers by today's anti-union forces. Their main targets are public employees and the pensions and other benefits they won in past bargaining with their government employers.
The governments' aim, of course, is to use the savings from that to make up for budget shortfalls resulting from the recession and, in many cases, from poor government management.
But there's another important reason: Public employees have become the vanguard of the labor movement. Their numbers and the percentage of them belonging to unions have been growing steadily, while the number and percentage of unionized workers in private employment have been shrinking.
That's caused anti-union forces to shift their major efforts into attempting to curb the escalating spread of unionization among public employees.
Which explains what's happening in Wisconsin, where Republican Gov. Scott Walker has moved to all but eliminate the bargaining rights of most state employees.
Walker is pushing bills through the GOP-controlled Legislature that would bar state employees from bargaining on anything except their pay, and limit any pay increases to the level of Consumer Price Index increases.
Employees would have no say in determining their benefits or working conditions, although most would have to increase their contributions to pension and health care funds by up to 50 percent. What's more, their contracts would have to be re-negotiated yearly, and union dues could no longer be deducted from employee paychecks. It's hard to imagine a union surviving under such restraints.
The pay and benefits of Wisconsin state workers may be too high, or too low, depending on who's measuring. But that could be addressed through negotiations between Gov. Walker and union representatives. But like some petty dictator, Walker insists, "I don't have anything to negotiate."
Peaceful negotiations are how it's done in civil societies, but that's not the style of union-busting Walker and his cohorts. And if anyone doesn't like Walker's approach, look out! He's alerted the National Guard to be armed and ready should Wisconsin state workers strike, disrupt state services or otherwise rise in protest.
Shades, again, of the 1930s. In fact, the last time the Guard was called out to quell a labor dispute in Wisconsin was during a United Auto Workers strike in 1934.
Workers eventually won that and many other struggles of the thirties, thanks to their courage and fierce determination and the broad public support they inspired. And that's precisely what it will take to overcome today's anti-worker onslaught by Walker and others like him.
The good news  and it's very good news  is that such help is here and growing fast. Crowds of as many as 70,000 labor supporters have been gathering daily outside the Wisconsin State Capital in Madison to demand that Walker and his fellow reactionaries return to the 21st century.
But give Walker this: Like the anti-labor politicians of the 1930s, he has aroused public outrage that has brought important new strength and solidarity to the cause of working people and their unions nationwide.
Certainly they'll need all the strength they can muster, with major efforts similar to Walker's in Wisconsin underway in at least 17 other states. In more than a dozen. , Republican anger over labor's strong support for Democrats in last year's elections have led directly to measures curbing union political activities.
President Obama is correct. There is indeed a nationwide "assault on unions." But as the assaults increase, so will the public outrage that's winning unions the broad support they so badly need  and so richly deserve.


Free user can take one test per day and valid for 2 days only.
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The pupose of Question Bank and Self Assessor is to build your basics step by step and not to go directly to exam specific topicwise or unit tests. The same are dealt in separate module.
TestBag has a unique and flexible Self Assessor which allows every user to create Self Tests for Formative Assessment (Assessment for Learning).
Learning can be effectively undertaken when you understand what is known to you, what remains to be known and initiate steps to bridge the gap. You require a system to apprise you the unknown or gap in your knowledge each topicwise. That is where Self Assessor steps in.
In this way of Self Assessment, the Learner is not spoon fed but has to look up to cover the unknown knowledge. Quite a good number of Learners may not prefer this slightly difficult way of Learning. The question is not of preference but of effectiveness. We remember the things we have had to look up ourselves rather than those were told.


text:
Marvels of Modernism: Mill Creek Canyon Earthworks
As a Bauhaus master, Herbert Bayer's career was dedicated to integrating artistic concerns into the everyday operations of society.
With the Mill Creek Canyon Earthworks, he created a much loved public park, stormwater detention dam, and Modernist masterpiece. A series of sculpted spaces that feel both ancient and modern, the Earthworks' pure forms—cones, circles, lines, and berms—are built into the alluvial delta at the mouth of Mill Creek Canyon. Grass and concrete, a wood bridge and steps: these are the materials at work, joined by the natural forces of Mill Creek itself. Installed in 1982, the Earthworks were immediately lauded for their fusion of art and infrastructure. Today, the same issues that necessitated building the Earthworks 25 years ago have dramatically intensified.
> View Online Exhibit


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Now, if defensive back Tremon Smith can perform anything like Tyreek Hill when he steps onto the field for the Chiefs' preseason opener against Houston on Thursday night, general manager Brett Veach and coach Andy Reid will have hit on something special at a position of tremendous need.
Then there's that speed — that world-class, can't-catch-me speed.
Either way, that's some serious speed.
The popular Madden video game even acknowledged Hill's wheels this year, when it granted him a 98 on its 1-to-100 scale for speed, making him the league's fastest player.
Speaking of Hester, the longtime Bears special teams dynamo, he's one of several players Chiefs special teams coach Dave Toub has been showing Smith on video. Toub also tutored Hester in Chicago and thinks Smith has the instincts and, yes, top-end speed to have a similar impact.
The Chiefs were taking a flier on Smith by selecting him in the sixth round, clearly reasoning his speed alone made him a worthwhile gamble. But he's also turned some heads on defense, working his way into the mix with the second team at a position that could be crucial to Kansas City's success.
"I think he's going to be a really interesting guy there," defensive coordinator Bob Sutton said.
That shouldn't necessarily come as a surprise. Smith picked off 15 passes over four years at Central Arkansas, even though teams rarely threw his direction. He also held his own against Power Five schools, picking off a pass against Oklahoma State in 2015 and leading Central Arkansas in tackles against Kansas State — his team's only loss before the FCS playoffs last season.
As you'd expect, he's doing it fast.
NOTES: LBs Reggie Ragland (knee) and Anthony Hitchens (hamstring) took part in some of Monday's practice, working together for the first time in camp. … WR Sammy Watkins left practice early with a hip issue, though the extent of it is unclear. OL Dillon Gordon left with a shoulder injury.


International Day of Sport for Development and Peace on April 6th!
OTTAWA, CANADA (April 4, 2014) – Right To Play President and CEO Johann Koss gathered with Athlete Ambassadors and representatives of the Government of Canada at École Secondaire Publique Louis-Riel in Ottawa today for an early celebration of the first-ever International Day of Sport for Development and Peace, to be observed annually on April 6.
The event was marked by the announcement from Canada's Minister of International Development and La Francophonie, Hon. Christian Paradis, of a new $5.3 million commitment from the Canadian government to support the Right To Play project: Advancing Health, Education and Development for Children and Youth (AHEAD) in West and Francophone Africa.
Right To Play was joined in Ottawa by Athlete Ambassadors and Canadian Olympians Rosie MacLennan (2012 London gold medallist) and Philippe Marquis (2014 Sochi men's freestyle skiing), Ottawa—Orléans Member of Parliament Royal Galipeau, and more than 30 local students.
The AHEAD project represents a one-year investment that will help Right To Play reach more than 235,000 children through critical play programs in Benin, Ghana, Liberia, Mali and Rwanda. It follows on a six-year (2007-2013), $20 million investment by the Canadian government for the Play To Learn program in West and Francophone Africa, as well as a $5 million commitment announced in January to establish Right To Play's three-year Learning, Empowerment and Play project in Jordan, which provides educational support to local children and communities affected by the Syrian Crisis through play.
Right To Play is a global organization that uses the transformative power of play to educate and empower children facing adversity. Through playing sports and games, Right To Play helps children in more than 20 countries to build essential life skills and better futures, while driving lasting social change. Founded in 2000 by four-time Olympic gold medallist and social entrepreneur Johann Olav Koss, Right To Play is headquartered in Toronto, Canada and has national offices in Canada, the Netherlands, Norway, Switzerland, the United Kingdom, the United States, and regional offices in Africa, Asia, the Middle East and South America. Our programs are facilitated by 600 international staff and more than 13,500 volunteer Coaches.


text:
Q: Showing enum value in column in database (Entity Framework 6) Is there a way to show the value in the database? EF (code-first) turns the column type automatically to integer and when trying to change the column type to nvarchar, it throws an exception saying the type is not compatible...
Is there a way to convert to the enum value without making the property a string and altering the get/set?
Here are my class and enum:
public class Dog
{
    public int Id { get; set; }
    public string Name { get; set; }

    [Column(TypeName = "nvarchar")]
    public Breed breed { get; set; }
}

public enum Breed
{
    Mix = 0,
    Breed1 = 1,
    Breed2 = 2,
}

Here is the type changing code:
protected override void OnModelCreating(DbModelBuilder modelBuilder)
{
    modelBuilder
         .Entity<Dog>()
         .Property(e => e.breed).HasColumnType("nvarchar");
}

I tried to change the column type and I expected EF would save the value as string and not as number.

redpajama_set_name: RedPajamaStackExchange


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We want to find some one that waiting about amazon listing product description translation,our company mainly sells waist trainer,sauna suit, we will send ...some one that waiting about amazon listing product description translation,our company mainly sells waist trainer,sauna suit, we will send English description , and need to translate to Italian.


One of the less announced setbacks of Donald Trump's duty talk has been metals costs.
Having contacted $3.30 per pound in June, copper currently sits at $2.75, a fall of somewhere in the range of 15%. Zinc, as well, has gotten down around 20% in a similar period.
At that point there are the valuable metals, the subject of the present Money Morning – as though financial specialists in this part required another kick in the face!
Astuteness has it that the late spring months – June, July and August – are the best season to purchase valuable metals (and their related stocks) with a view to offloading the accompanying winter or in late-winter.
It's one of those exchanges that appears to work better in the back view reflect than it does continuously, nonetheless.
In the event that you glance back at an outline of gold you can as a rule locate a low at some point in July, and afterward discover a point between the next October and April, where the gold cost was 10% or 20% higher, and after that pronounce that the exchange worked.
Purchasing the low and offering the high continuously is a fairly trickier recommendation. All things considered, it is do-capable.
Notwithstanding, gold itself is at present in freefall. In April, gold was re-trying five-year highs at $1,360-$1,370 per ounce. There was a pleasant uptrend set up. Each low was higher than the last. Discuss expansion was doing the rounds once more, and the arrangement was gleaming, yellow-y metal.
Presently it is some $130 bring down at $1,227. Each low is lower than the last. Each endeavor at a rally is frail. The pattern is solid and the pattern is down. To purchase now and endeavoring to play the "late spring exchange" is to attempt and catch a falling blade. At times it works and the group of onlookers praises – anyway the danger of self-damage is high.
Tuesday was especially fierce. Gold's adversary number one, the administrator of the Federal Reserve Bank, Jerome Powell, said that the economy was developing at a "strong pace", that the joblessness rate was required to fall further, that the ongoing pickup in expansion, around the Fed's 2% target, was "empowering".
The Fed has officially raised financing costs twice this year and Powell penciled in two more quarter-point moves. Stocks appropriately mobilized (a bit), the dollar aroused – and gold took a $20 clobber in the face, sending it to two-year lows.
My 17-year-old child, who is in his first year of A-levels, is pondering what he needs to improve the situation a living. I'm enticed to instruct him to end up a silver sales representative.
You're offering a wonderful item that has a gazillion diverse employments. Any individual who handles it is immediately enthralled. Human impulse reveals to you it's valuable.
What's more, it has the absolute most convincing venture stories of all behind it – from a controlled market that is going to explode and send silver to the moon; to a fiat cash framework that is going to explode and send silver to the moon; to different innovative uses that will require so substantially silver that they will, truly, send silver the moon.
However, I'm not upholding that he turn into a bullion merchant. Or maybe, he ought to do what JP Morgan does. Offer silver. Short it. Since all it ever appears to do is go down. You can bring home the bacon doing it. Individuals do.
There are brief snapshots of relief once in a while. At that point the offering resumes.
Silver has been enduring the one-two punch recently. It's being sold in light of the fact that it's a valuable metal and it's being sold on the grounds that it's a modern metal. The most exceedingly awful performing stocks among the mineworkers on Tuesday's day of slaughter were, yes, the silver diggers.
The present cost is $15.42 per ounce. If it somehow happened to go anyplace close to its verifiable midpoints – a silver dollar (one ounce) is multi day's wage for a working man, and all that – it ought to be, I don't have the foggiest idea, five or ten times its present cost.
Rather, right now, it is gazing intently at the barrel of its 2015-16 lows of around $14.
Would it be a good idea for you to feel the dread and dive in any case?
So do you go up against the mid year exchange? Even with this bearishness – for sure, this article is most likely a contrarian pointer in itself – do you pull out all the stops, and purchase valuable metals?
There are a few motivations to do as such. The market is oversold, by pretty much any measure you want to utilize. Bearish slant and antagonism is all over. Purchasing plunges in the mid year can demonstrate fulfilling.
Ross Norman of bullion dealer Sharps Pixley reports that his organization "beginning to see great physical offering at these record multi month gold lows, when one may customarily expect deal chasing". This would propose we are near some sort of definite capitulation.
"The uplifting news for gold bulls," Norman proceeds, "is that the weaker turns in the ETFs have sold out, the theoretical long shade on CME has everything except vanished and we have consumed around 700 tons of utilized offering (and we are currently at levels not seen since mid 2016), while the interest for physical announced by the Mints the world over are at generational lows. Indian request is sketchy and Chinese request just sufficient. I may include that the expression "purchase gold" on Google Trends has recently slipped to 10 years low." at the end of the day, there is a considerable measure of space for purchasers to return to the market.
Numerous valuable metal excavators have really been showing relative quality and the proportion amongst mineworkers and gold is, trust it or not, in an uptrend. That is ordinarily a positive sign. The offering won't keep going forever, regardless of whether it senses that it will. Valuable metals' chance will come back once more. Shortage spending in the US is rising further. Mining stocks are shoddy.
Then again, what is oversold can get more oversold. Negative feeling can get more negative. The "season" exchange is unreasonable. What's more, who cares what the mining stocks are doing?
The shortfall spending story, regardless of being continuous, just appears to issue a portion of the time. What's more, regardless of whether mining stocks are shoddy, they can get significantly less expensive. Et cetera.
This is an example of the twirl of logical inconsistencies that possess large amounts of a market – like valuable metals – which is going no place. Back in the positively trending market long stretches of 2001-11, everything appeared to be so much clearer. Presently gold and silver are, best case scenario, run bound. Even from a pessimistic standpoint, the bear showcase is back on. I can see bolster for gold at $1,200, at $1,120 and – paradise preclude it ought to go that low – at $1,050.
My hypothesis on gold has for quite a while been that out not too far off things are gradually arranging for gold – expansion, credit emergencies, financial frenzy, and the remainder of it – yet the ducks are not yet in line. Multi day they will be, however that day has not yet come. At the end of the day, we are not yet in a positively trending market.
It may be that when the positively trending market comes, things will move so rapidly you won't have sufficient energy to get situated – that is the Jim Rickards hypothesis – so it sounds good to claim some at this point. In five years, gold purchased at $1,225/oz may look a sound venture.
In any case, in the shorter-term, you chance getting a falling blade. The easy way out, for the time being, is down. It will remain so until the point when so much tax discussion settle.
Unemployment Is Low and the Economy is Booming, so Why Is Trump Looking for More Trade Wars?


text:
Shantanu Basu (born 1964) is an American astrophysicist and Professor in the Department of Physics and Astronomy at the Canadian University of Western Ontario, in London, Ontario.

Career

Basu received his PhD in Physics from the University of Illinois at Urbana-Champaign in 1993, and held academic positions at Michigan State University and the Canadian Institute for Theoretical Astrophysics, in Toronto, before joining Western in 1999. Basu has made contributions to understanding the fragmentation of interstellar molecular clouds, the role of magnetic fields and angular momentum in gravitational collapse and star formation, the origin of luminosity bursts from young stellar objects, and the origin of power-laws in the mass distribution of stars. He is one of the originators of the Migrating Embryo Model for protoplanetary disk evolution, which is a unified scenario for angular momentum transport, binary star and giant planet formation, and the formation of ejected freely floating low mass objects.

Awards and honors

Asteroid 277883 Basu, discovered by Canadian astronomer Paul Wiegert at the Mauna Kea Observatories in 2006, was named in his honor. The official  was published by the Minor Planet Center on September 19, 2013 ().

References

External links

 The Migrating Embryo Model for Disk Evolution, Shantanu Basu, Eduard Vorobyov (2012)

1964 births
Living people
21st-century American astronomers
University of Illinois Urbana-Champaign alumni
Michigan State University faculty
Academic staff of the University of Toronto

redpajama_set_name: RedPajamaWikipedia


Makoto FujimuraMakoto Fujimura was born in 1960 in Boston, Massachusetts. Educated bicultural between the United States and Japan, Fujimura graduated from Bucknell University in 1983 and received an M.F.A. from Tokyo National University of Fine Arts and Music as a National Scholar in Nihonga (Japanese-style painting) in 1989. His thesis painting was purchased by the university and he was invited to study in the Post–M.F.A. lineage program, a first for an outsider to this prestigious traditional program. During his years in the program, he experienced "a transfer of allegiance from art to Christ." His book River Grace traces his journey of mastering Nihonga technique, using carefully stone-ground minerals including azurite, malachite, and cinnabar, along with his deep wrestling with art and faith issues.
In 1992 he became the youngest artist ever to have had a piece acquired by the Museum of Contemporary Art in Tokyo. Public collections include The Saint Louis Museum, Museum of Contemporary Art in Tokyo, and the Time Warner / AOL / CNN building in Hong Kong. His paintings are represented by Dillon Gallery in New York and in Tokyo.
Fujimura was appointed to the National Council on the Arts, a six-year presidential appointment, in 2003. WORLD magazine honored him as its Daniel of the Year in 2005.
In 1990 Fujimura founded The International Arts Movement, an arts advocacy organization that wrestles with the deep questions of art, faith, and humanity. Fujimura has served as an elder at Redeemer Presbyterian Church as well as a founding elder at The Village Church, both Presbyterian Church in America congregations in New York City. His writings on art and faith issues have appeared in Image Journal , Books and Culture , American Arts Quarterly , and WORLD magazine.


This is a beautiful, sensuous but a controversial semi-autobiographical story about a 15 year old teenage girl who was physically and emotionally abused by her mother and elder brother. She felt unable to control her predicament.
She sought solace and control through her passionate affair with a wealthy Chinese man (actor Tony Leung) from Cholon. However, the affair is tragic from the very beginning because of the cross-cultural conflicts experienced and endured by the two lovebirds.
There is on one hand, the French social restrictions about relationships with the "inferior" race of Vietnamese and the Chinese. On the other hand, it was about the Chinese tradition of arranged marriages.
Marguerite Duras Books Note: the views expressed here are only those of the reviewer(s).


Various semi-automatic and revolver handguns are discussed.
This post is meant to provide a very brief review of the "Flash Bang" holster. There are a multitude of reviews and videos on this innovative holster and I'll provide a few links at the end of this entry.
A previous post happily shared my purchase of the new "baby Glock" – the Glock 42, chambered in .380. I started carrying my new "baby" in a pocket holster that I kept in a zippered pocket of my coat or in my purse. While that allowed me to carry the firearm "with" me, it didn't provide a method of carrying it "on" me, which is the preferred method for self defense.
The "Flash Bang" is a molded kydex holster, shown here with the longest of the snap on suede straps that attach at the midpoint of the bra, between the cups. The holster cradles the G42 and covers the trigger.
The gun "snaps" in place and then tucks up under the underwire of your bra.
To draw the gun, you grasp the handle and pull down quickly to release it.
I changed out the suede strap (shortest of the three) that came with the holster, and the directions are serious when they warn you to watch for "small parts" as you do this. Mission accomplished, I then attached the holster by snapping the VERY strong one way snap onto my bra, without a gun in it at first, just to get the feel of it.
Next I put the gun in the holster, you have to put it in the holster with a bit of "authority" for it to snap in. For this initial test I did it without the magazine installed- which I wouldn't advise you to try with this model. There are some "sharp-ish" edges at the base of the grip that will not feel comfortable, particularly while sitting. After I put in an empty magazine it immediately felt better!
My final stage of "fitting" was with a fully loaded magazine (although not brave enough to have one in the chamber at this point! ). The added weight pulled down a bit on the bra, and I made some adjustments. I found it fit my frame a little better to "tweak" it so the muzzle pointed a little down.
The second day I wore it under a thin pullover shirt, and it was well concealed. You would have to know that it was there and be looking for it. Within a very short amount of time, I mostly forgot it was there.
The "mature woman" in me found some things a little uncomfortable. Kydex is a hard material, and between my aging and thinning skin and the effects of gravity "at work" on my anatomy, there were a few "pinch spots" that I would feel occasionally while wearing it.
I decided what was needed was a "holster cozy." My husband -the creative master- jumped on that project before I even had a chance to think about materials for it, and literally within minutes presented me with a "cozy" from an old sock.
He was ready to permanently attach it to the Kydex holster, and I was appalled.
Another "fascinating" experience of getting to be an old woman are "hot flashes." The placement of this holster is in an area that, pardon me, can on occasion get pretty "damp." Whatever was used for the "cozy" had better be able to be thrown in the washer!
This "cozy" did improve the comfort of the holster, and is completely washable.
Here is the "cozy" laid out flat. Any soft, absorbent, washable material would do, and I am sure the truly crafty could add embellishments and "prettify" it, but it works for me! Just be sure that you leave the bottom opening of the holster clear so you don't get it tangled up when holstering/ drawing your gun!
A few links for reviews: pro and con !


Not for the timid and not for the tame, A Boy & A Girl are an EDM outfit based out of Hollywood, CA. Recently discovered by Diplo's record label Mad Decent and Dillon Francis, their wild synth lines and massive sub bass have exploded throughout the music community - flooding festivals like Electric Daisy Carnival and Ultra Miami, as well as the hottest dance clubs in America like Exchange LA and Avalon. In addition to breaking out with an official remix of Dillon Francis and NGHTMRE's hit "Need You," a remix of their song "Stampede" featuring Armanni Reign and Reid Speed was included in Excision's massive 2016 Shambhala Mix. With other releases on Big Beat/Atlantic and Play Me Records, A Boy & A Girl are prepping for a busy 2017 packed with shows, festivals, and collaborations.


Civil society has been working for years on participation, transparency, accountability and governance issues. Plenty of newer initiatives (small and large) look at new technologies as a core tool in this work. But are these groups talking and learning from each other?