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text:
Q: How do I retrieve a file from a SQL Server database? I have successfully uploaded files into my SQL Server database. I can bring back the information into a GridView. I am unable to figure out how to create a hyperlink to actually open the file.

A: You need to create an URL that handles the pictures and returns the DB content into the response stream. As it happens at SQL Saturday #26 I had a presentation that showed exactly this. You can doaloand my slides from the link, go into Demo 2 and in the lotsOfPictures solution you'll find Picture.aspx.cs, that does exactly what you ask for:
using (SqlConnection conn = new SqlConnection(connStr))
            {
                conn.Open();

                SqlCommand cmd = new SqlCommand(
@"SELECT picture
FROM resized_pictures
WHERE picture_id = @id
AND picture_size = @size;", conn);
                cmd.Parameters.AddWithValue("@id", pictureId);
                cmd.Parameters.AddWithValue("@size", size);

                using (SqlDataReader rdr = cmd.ExecuteReader(
                    CommandBehavior.SequentialAccess))
                {
                    if (rdr.Read())
                    {
                        Response.ContentType = "image/jpeg";
                        byte[] bytes = new byte[1024];
                        long offSet = 0;
                        int countRead = (int) rdr.GetBytes(
                            0, offSet, bytes, 0, 1024);
                        while (countRead > 0)
                        {
                            Response.OutputStream.Write(bytes, 0, countRead);
                            offSet += countRead;
                            countRead = (int)rdr.GetBytes(
                                0, offSet, bytes, 0, 1024);
                        }
                    }
                }
            }

The important pieces of the puzzle are the SequentialAccess flag passed to the SqlCommand reader that will return a true stream, so the page does not load the whole image in memory before returnning. For a high performance server you should use async operations, like described in Asynchronous Pages in ASP.NET 2.0.

A: Have not tried this myself, but how about streaming the data into a temporary file on the local file system and then providing a link to that temporary file?

A: Normally you would use your server side code to send the appropriate headers, then just echo the content.
From the PHP manual:
// We'll be outputting a PDF
header('Content-type: application/pdf');

// It will be called downloaded.pdf
header('Content-Disposition: attachment; filename="downloaded.pdf"');

// The PDF source is in original.pdf
readfile('original.pdf');

A: If your file is stored in the database, you are probably storing it as a blog or byte array.  On the hyperlink click event, you will need to pass the byte array into a stream, and use a stream writer to create the file.  Then execute the file.

redpajama_set_name: RedPajamaStackExchange


text:
Q: ShutdownHook code not being executed on System.exit(0) I have Shutdown hook that i attach to runtime
Runtime.getRuntime().addShutdownHook(new ShutDownHook(false));

Here is a shutDownHook Class
public class ShutDownHook extends Thread {

    private final boolean interupt;

    public ShutDownHook(boolean interupt) {
        this.interupt = interupt;
    }

    @Override
    public void run() {

        if (interupt) {
            return;
        }
        System.out.println("ShutdownHook Execution");
        DbUtil.insertIntoDailyStats(MainDataModel.downloadedBytesSessionProperty().getValue());
        MainDataModel.getInstance().loginProfile.getPreferences().putLong(
                Info.PreferenceData.PREF_USER_DAILY_STAT_DOWNBYTE, MainDataModel.downloadedBytesTodayProperty().get());

         System.out.println("ShutdownHook Execution finished");

    }

}

And i close my application from System tray icon with a method
 exit.addActionListener((ActionEvent e) -> {
            try {
                GlobalScreen.unregisterNativeHook();
                System.exit(0);
            } catch (NativeHookException ex) {
                ex.printStackTrace();
            }
        });

Application closes bud hook execution didnt went thru, any idea why?
I know there are cases when ShutdownHook doesnt execute bud im closing my application with System.exit(0); that shoud be all safe and sound?

A: Ok i found a problem i had multiple ShutDownHooks hooked in for some reason this one didnt executed , i removed all beside one and now everything works ok.Maybe too much of a load.
Works flawlessly , also if you use netbeans dont use RED TERMINATION BUTTON , - just a note.That way you never get execution of SDH.


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text:
\section{introduction}

Quantum coherence is widely regarded as an essential resource \cite{Streltsov:17} for quantum information processing \cite{Ladd:10}, quantum sensing  \cite{Degen:17}, and quantum interferometry \cite{Cronin:09}. The inevitable interaction of quantum systems with an external environment is generally believed to lead to the decay of quantum coherence in a process known as decoherence \cite{Schlosshauer:97}. As decoherence upsets the unitary time evolution necessary for the successful operation of quantum bits and sensors, understanding and controlling decoherence mechanisms is a key research goal of quantum science and technology.

An additional motivation to study decoherence comes from recent experimental and theoretical studies  of quantum effects in biological processes, such as photosynthetic energy transfer \cite{Cheng:09,Pachon:12,Brumer:18}, vision \cite{Tscherbul:15a,Dodin:19},  and avian magnetoreception \cite{Hiscock:16}. These studies have indicated that non-trivial quantum effects such as coherence and entanglement \cite{Cheng:09,Pachon:12} can persist under noisy conditions typical of biological environments at room temperature. In all of the experimental studies performed to date, quantum coherence was introduced into the system by means of coherent (ultrashort) laser pulses \cite{Cheng:09,Pachon:12,Brumer:18}. However, biologically relevant photosynthetic light-harvesting is driven by natural sunlight, which is an incoherent mixture of number states,  raising an important question: Can excitation by incoherent light alone generate coherence in multilevel quantum systems \cite{Brumer:12,Tscherbul:14,Tscherbul:15,Cao:14,Dodin:16,Dodin:16a,Brumer:18}?

Surprisingly, the answer to this question is ``yes'', although the coherences are distinctly different from coherent light-induced effects \cite{Dodin:19}. Incoherent radiative transitions between manifolds of closely spaced energy levels can interfere to produce {\it noise-induced Fano coherences} in multilevel atomic and molecular systems even in the absence of coherent driving \cite{Agarwal:70,Fleushhauer:92,Hegerfeldt:93,Kozlov:06,Tscherbul:14,Tscherbul:15,Dodin:16,Dodin:16a,Koyu:18}.
The interference manifests itself  through the cross terms in the quantum optical (Bloch-Redfield)  master equation, which correspond to the interaction of a common incoherent light mode with the  dipole moments of the transitions from the same initial state to different final states \cite{Kozlov:06,Tscherbul:14,Dodin:16,Dodin:16a,Koyu:18}.

Initial theoretical studies of Fano coherences highlighted their significance in the context of lasing without inversion \cite{Fleushhauer:92} and quantum jumps in trapped ions \cite{Hegerfeldt:93}.  Agarwal and Menon \cite{Agarwal:01} explored the conditions under which the three-level V-system (see Fig. 1) pumped by  incoherent light  approaches  thermodynamic equilibrium in the long-time limit. They showed that in the absence of symmetry between incoherent pumping and spontaneous decay, non-trivial steady-state coherences can arise, leading to non-equilibrium steady states.  Kozlov, Rostovtsev, and Scully \cite{Kozlov:06}  showed that incoherent pumping of the V-system with degenerate upper levels can create  coherent population-locked states, which depend on the initial state of the system \cite{Kozlov:06}.  Recent theoretical work by Dorfman, Scully, Mukamel, and co-workers \cite{Scully:11,Dorfman:13} reinvigorated  interest in noise-induced Fano coherences by showing that they can enhance the efficiency of quantum heat engines by breaking the principle of detailed balance.  Note, however, that a  problem has recently been discovered \cite{Creatore:13} with the master equation approach used in Refs.~\cite{Scully:11,Dorfman:13} which gives negative population dynamics at long times.

We have explored the dynamical properties of Fano coherences in realistic V-systems with nondegenerate excited states, establishing the existence of two dynamical regimes depending on the ratio of the excited-state splitting $\Delta$ to the radiative decay rate $\gamma$ \cite{Tscherbul:14,Dodin:16,Koyu:18}. In the underdamped regime characterized by $\Delta/\gamma\gg 1$, Fano coherence exhibit damped oscillations that decay on the timescale $\tau\simeq 1/\gamma$ \cite{Tscherbul:14,Dodin:16}. In the overdamped regime, where the excited-state splitting is smaller than the radiative decay rate, we observe long-lived quasisteady-state coherences with the lifetime $\tau=\frac{2}{\gamma}(\frac{\Delta}{\gamma})^{-2}$ \cite{Tscherbul:14,Dodin:16}. We have also explored the dynamics of the V-system driven by polarized incoherent light \cite{Dodin:18} and proposed an experimental scheme for observing noise-induced coherence dynamics in Calcium atoms driven by incoherent radiation.

The majority of theoretical studies of noise-induced Fano coherences have focused on the dynamics induced by {\it isotropic} incoherent light, whose polarization ($\bm{\epsilon}_\lambda$) and propagation ($\mathbf{k}$) vectors point randomly in all directions. The coherence properties of isotropic incoherent light [such as its first-order degree of coherence $g^{(1)}(\tau)$] are  independent of $\bm{\epsilon}_\lambda$  and $\mathbf{k}$ \cite{Mandel:95}. As a consequence,  the  light-matter interaction only depends on the angles between the  dipole moment vectors $\bm{\mu}_{ij}$ and $\bm{\mu}_{kl}$ for radiative transitions between the system eigenstates $|i\rangle \leftrightarrow |j\rangle$ and  $|k\rangle \leftrightarrow |l\rangle$  \cite{Tscherbul:15}. The resulting quantum master equation treats   incoherent excitation and decay dynamics on an equal footing, leading to the decay of quantum coherences in the long-time limit and the establishment of the canonical equilibrium steady state \cite{Agarwal:01}, although the time it takes to reach this state can be extremely long for nearly-degenerate levels \cite{Tscherbul:14,Dodin:16,Koyu:18}.

In contrast, when a quantum system is excited by polarized incoherent light, only one polarization mode of the light interacts with the transition dipole moment vectors \cite{Dodin:18,Dodin:19}, whereas spontaneous emission still occurs in all directions (in the absence of an external cavity).  As a result of the imbalance between incoherent pumping and spontaneous emission, the excitation with polarized incoherent light can lead to the emergence of nonequilibrium steady states (NESS) featuring  coherences  in the energy eigenstate basis and populations deviating significantly from their expected canonical values \cite{Agarwal:01}.
We note that these steady states are distinct from the more commonly occurring NESS that arise due to the additional selection rules for excitation with polarized light. For instance, the $\Delta m_J=\pm 1$  electric dipole selection rule implies that the $|J=1,m_J=0\rangle$ excited state cannot be populated from the ground $|J=0,m_J=0\rangle$ state irradiated by incoherent light polarized in the $x$-direction \cite{Dodin:18}. While important for optical pumping, these NESS manifest themselves through the appearance of dark states, and do not feature coherences in the energy eigenstate basis of the system, so we will not consider them further in this work.

In contrast to the case of excitation with isotropic incoherent light, very little attention has been devoted to the NESS and steady-state Fano coherences induced  by polarized incoherent excitation of multilevel quantum systems. Agarwal and Menon  derived analytical expressions for steady-state Fano coherences in a three-level V-system driven by broadband incoherent radiation \cite{Agarwal:01}. We have shown that the steady-state coherences can occur in  Calcium atoms driven by polarized  incoherent light \cite{Dodin:18}. However, even the most basic properties of steady-state Fano coherences  (such as their dependence of the system and excitation parameters, and their sensitivity to decoherence)  remain unexplored, despite widespread occurrence of polarized sunlight in nature \cite{Cronin:11}, and the resultant possibility of  noise-induced coherences playing a role in biological excitation processes.

Here, we present a theoretical analysis of steady-state Fano coherences in a three-level V-system driven  by polarized incoherent excitation. The V-system serves as a minimal model, in which to study the quantum dynamics of noise-induced coherence generation \cite{Tscherbul:14,Cao:14} and energy transfer \cite{Kassal:14,Cao:14,Tscherbul:18}.  We obtain analytic results for the steady-state coherences and explore their dependence on the system parameters. Our results suggest that the coherences are  maximized when the excited-state splitting is small compared to the radiative decay rate ({\it i.e.}, in the large-molecule limit \cite{Tscherbul:14}).
We clarify the physical origin of the coherences by establishing an equivalence between the quantum master equation describing the V-system excited by polarized incoherent radiation and that describing the dynamics of non-equilibrium heat transport across a pair of quantum two-level systems (qubits) coupled to two independent thermal baths \cite{Li:15}. Finally, we present an experimental scenario for observing the  signatures of steady-state Fano coherences in the fluorescence signal emitted by calcium atoms excited by polarized incoherent light.
Our analysis paves the way toward further theoretical and experimental studies of NESS and steady-state Fano coherences in thermally driven atomic and molecular systems, and for the exploration of their  potential role in natural processes  induced and sustained by solar light.

In the rest of this paper, we will present the details of our theoretical calculations based on the nonsecular Bloch-Redfield (BR) quantum master equation (Sec. II). In Sec. III we report the results for steady-state Fano coherences as a function of the system and excitation parameters. In Sec. IIIA we establish the physical basis for steady-state Fano coherences using a two-bath transport model. The effects of relaxation and decoherence are examined in Sec. IIIB. An experimental proposal for observing Fano coherences in Calcium atoms in put forward  in Sec. IV. Section V summarizes  and discusses the main results of this work.

\section{Theory and Methods: Analytical solutions to Bloch-Redfield equations in the steady state}

To model the quantum dynamics of the V-system driven by polarized incoherent radiation, we use the Bloch-Redfield (BR) quantum master equation for the system's density matrix  in the eigenstate basis \cite{BPbook,Agarwal:01,Tscherbul:14,Dodin:16,Dodin:16a}
\begin{align}
    \Dot{\rho}_{ii} &= -(r_{i}+\gamma_{i}+\Gamma_i) \rho_{ii} + r_{i} \rho_{gg} - \sqrt{r_{a}r_{b}} \rho^{R}_{ab} \nonumber
    \\
    \Dot{\rho}_{ab} &= -\frac{1}{2}(r_{a}+r_{b}+\gamma_{a}+\gamma_{b}+2\gamma_{d})\rho_{ab} -i\Delta \rho_{ab} + \sqrt{r_{a}r_{b}} \rho_{gg} - \frac{1}{2} \sqrt{r_{a}r_{b}} (\rho_{aa}+\rho_{bb}) \label{QME1}
\end{align}
where $\rho_{ab}=\rho^{R}_{ab}+i\rho^{I}_{ab}$ is the coherence between the excited eigenstates $\ket{a}$ and $\ket{b}$ [see Fig.~\ref{fig:1}(a)], $\gamma_i$ is the spontaneous decay rate of the $i$-th excited-state level,  $r_i = \bar{n} \gamma_i$ is the incoherent pumping rate, and  $\bar{n}=[1-e^{\hbar\omega_{ag}/{kT}}]^{-1}$ is the average photon occupation number of the incoherent radiation filed, which we assume to be polarized in the $x$-direction of the space-fixed coordinate frame \cite{Dodin:18}.  The environmental relaxation and decoherence channels (to be considered  in Sec. IIIB) are described by the phenomenological rates $\Gamma_i$ and $\gamma_d$.  Note that Eq. (\ref{QME1})  assumes that  non-radiative coupling with an external  environment ({\it e.g.} phonons) cannot generate coherence between the eigenstates of the V-system \cite{Benenti:17}, {\it i.e.}, that Fano coherence can only be generated by the light-matter interaction through the $ \sqrt{r_{a}r_{b}} \rho_{gg} $ term in Eq. (\ref{QME1}). Isotropic incoherent excitation in the presence of coherence-generating system-phonon interactions have been considered elsewhere \cite{Svidzinsky:11,Tscherbul:15,Tscherbul:18,Dodin:19}.

We will consider the case of a symmetric V-system with $\gamma_{a}=\gamma_{b}=\gamma$, $r_{a}=r_{b}=r$, and $\Gamma_{a}=\Gamma_{b}=\Gamma$ which contains all of the essential physics while drastically simplifying the analytical solution of the BR equations (\ref{QME1}).
Imposing the trace conservation condition for the ground-state population $\rho_{gg}= 1-2\rho_{aa}$, we obtain the BR equations for the symmetric V-system in the absence of environmental relaxation and decoehrence
\begin{align}
    \Dot{\rho}_{aa} &= -(3r+\gamma +\Gamma) \rho_{aa} - r \rho^{R}_{ab}+r  \nonumber \\
    \Dot{\rho}^{R}_{ab} &= -3r \rho_{aa} - (r+\gamma+\gamma_d)\rho^{R}_{ab} + \Delta \rho^{I}_{ab}+r \nonumber \\
    \Dot{\rho}^{I}_{ab} &= -\Delta \rho^{R}_{ab}-(r+\gamma+\gamma_d)\rho^{I}_{ab} \label{QME2}
\end{align}
Here, as above, the phenomenological  parameters $\Gamma$ and $\gamma_{d}$ account for the effects of relaxation and decoherence between the excited states of the V-system due to, {\it e.g.}, non-radiative processes. These effects will be explored in Sec. IIIB below.  In Sec. III, we will begin by considering only the radiative processes, setting $\Gamma=\gamma_{d}=0$.

The BR quantum master equations (\ref{QME2}) can be rewritten in matrix-vector notation as \cite{Dodin:16}
\begin{equation} \label{state_vector_DE}
    \Dot{\mathbf{x}}(t) = \mathbf{A}\mathbf{x}(t) + \mathbf{d},
\end{equation}
where $\mathbf{x}(t)=[\rho_{aa}(t),\rho^{R}_{ab}(t),\rho^{I}_{ab}(t)]^{T}$ is the state vector in the Liouville representation \cite{Dodin:16}, $\mathbf{d}=[r,r,0]^{T}$ is the driving vector  corresponding to the V-system  being initially in the ground state [$\rho_{gg}(t=0)=1$], and the coefficient  matrix $\mathbf{A}$ is given by
\begin{equation}
    \mathbf{A} =
\begin{bmatrix}
    -(3r+\gamma) & -r & 0 \\
    -3r  & -(r+\gamma) & \Delta \\
    0 & -\Delta  &  -(r+\gamma)
\end{bmatrix}
\end{equation}
In this work, we are primarily interested in the steady-state behavior of the V-system irradiated by incoherent light. Setting $\Dot{\mathbf{x}}(t)=0$ in Eq. (\ref{state_vector_DE}) we obtain the steady state solution
\begin{equation} \label{SSVec}
    \mathbf{x}_{s} = - \mathbf{A}^{-1} \mathbf{d}
\end{equation}
The steady-state solution is unique only if the coefficient matrix $\mathbf{A}$ is non-singular, {\it i.e.}, $\det(\mathbf{A}) =3r^{2}(r+\gamma) -(3r+\gamma)[\Delta^{2}+(r+\gamma)^{2}] \ne 0$. The determinant is non-zero in general but  it tends to zero as $\Delta \to 0$ and $r/\gamma\to \infty$, leading to initial condition-dependent population-locked steady states  similar to those explored in Ref. \cite{Kozlov:06}. However, due to, {\it e.g.}, differential level shifts experienced by the excited levels interacting with the pumping field, most real-world V-systems will have $\Delta > 0$. As a result,  $\det(\mathbf{A}) \neq 0$ and  the steady-state solution  (\ref{SSVec}) is uniquely defined.

\section{Steady-state Fano coherences: Results and Discussion }

Substituting the inverse of matrix $\mathbf{A}$  into Eq. (\ref{SSVec}), we find analytical expressions for excited-state populations and the real part of Fano coherence  in the steady state  \cite{KoyuThesis:19}
\begin{align}
    \rho_{aa} &= \frac{r[\Delta^{2}+(r+\gamma)^{2}-r(r+\gamma)]}{(3r+\gamma)[\Delta^{2}+(r+\gamma)^{2}]-3r^{2}(r+\gamma)} \nonumber \\
    \rho^{R}_{ab} &= \frac{r\gamma(r+\gamma)}{(3r+\gamma)[\Delta^{2}+(r+\gamma)^{2}]-3r^{2}(r+\gamma)}  \label{SS_Dyn}
\end{align}
with the imaginary part of the coherence  $\rho^{I}_{ab} = -\frac{\Delta}{(r+\gamma)} \rho^{R}_{ab}$, in agreement with the results of Ref.~\cite{Agarwal:01}. Below we analyze the remarkable properties of  steady-state Fano coherences  not explored in Ref.~\cite{Agarwal:01}, and study  their dependence on  the excited-state splitting $\Delta/\gamma$ and the incoherent pumping rate $r=\bar{n}\gamma$.  The effects of relaxation and decoherence are considered in the following section.

First, we observe that neither the real nor imaginary part of the Fano coherence vanishes in the steady state, in contrast to the previously explored cases of incoherent driving with isotropic (unpolarized) light \cite{Tscherbul:14,Dodin:16,Koyu:18}. Figure~ \ref{fig:2}  shows the time evolution of excited-state populations and coherences in the V-system driven by polarized incoherent light. The results are obtained by numerical integration of Eq. (\ref{QME2}).
The equilibration timescale depends on the dynamical regimes of the V-system classified in our previous work \cite{Dodin:18,KoyuThesis:19}, which are determined by the value of excited-state splitting $\Delta/\gamma$ and the incoherent pumping rate $r=\bar{n}\gamma$.  Regardless of the transient dynamics,  the V-system eventually reaches a steady state characterized by nonzero values of  Fano coherences shown by the dashed lines in Fig.~ \ref{fig:2}, which are in excellent agreement with the analytical expressions (\ref{SS_Dyn}).

It may seem surprising that incoherent driving  excites a coherent superposition rather than an incoherent mixture of energy eigenstates.
The presence of coherences seems incongruent with an incoherent nature of the light source, which is thought of as having an entirely random phase at every instant.
For such a source excitations generated at different times will pick up a different phase from the fluctuating light field, yielding a random phase that vanishes upon averaging over the realizations of the incoherent source.
However, this phase averaging argument does not hold for excitations generated at the same instant.
In this case, both excitations will accrue the same (randomly selected) phase from the incoherent drive, resulting in an in-phase superposition of the two eigenstates.
That is, while the relative phase between excitations generated at different times is uncorrelated, the relative phase of simultaneous excitations is deterministic since both arise by interacting with the same state of the light field \cite{Dodin:19}.

To further understand the counterintuitive emergence of the coherent steady-state, we  consider the dynamics of the contributing coherent excitations.
As  noted  earlier in this section, an incoherent light source generates a coherent drive due to the presence of simultaneous excitations from the ground state to two different excited states.
This process generates an in-phase superposition of two energy eigenstates.
Once this excitation is generated, it undergoes unitary evolution, accruing a periodic relative phase with frequency $\Delta$.
Moreover, it will slowly dephase with rate $\gamma_d$ and relax to the ground state with rate $\gamma + r+\Gamma$ [see Eq.~(\ref{QME1})].
The timescales and effects of these contributions on the dynamics of a single excitation are shown schematically in  Fig.~\ref{fig:timescales_dephasing}(a).

In incoherent driving, the source is assumed to be continuously acting on the system, generating new excitations at every instant in time. At each instant, therefore, a new in-phase superposition is generated and undergoes the dynamics described above. The resulting ensemble dynamics are then obtained by summing over the contributions of all of these different excitations, as shown in Fig.~\ref{fig:timescales_dephasing}(b)
If the system frequency $\Delta$ is much larger than the excitation decay rate ($\sim \gamma$), then excitations generated at earlier times will have accrued some phase due to unitary evolution in the excited state manifold while new excitations will always produce an in-phase superposition.
Summing over these contributions then leads to an integral over different phases, producing an ensemble dephasing with excitations generated at different times carrying different phase that eventually averages to near zero.
However, when the frequency is much slower than the excitation lifetime, nearly all excitations will decay before accruing an appreciable phase.
As a result, nearly all excitations will be in the initially prepared in-phase superposition, leading to the previously reported quasi-stationary coherences \cite{Tscherbul:14,Dodin:16}.
Generally, the interplay of these different processes need not result in an incoherent steady state, as new coherent superposition may be refreshed quickly enough to maintain coherence in the long-time limit.

In the case of unpolarized excitation that obeys the fluctuation-dissipation constraint $r = \bar{n} \gamma$, the rate of generating new excitations $r$ and their decay rate $\sim$$\gamma$ are directly related.
This bound ensures that the delicate interplay of generating new excitations, their coherent evolution and subsequent decay are balanced to yield an incoherent thermal steady-state.
However, if these rates are allowed to vary independently, it becomes possible to generate residual coherences as the balance between these different processes is broken.
As discussed in the framework of the thermal transport model in Sec. IIIA below, polarized driving  breaks this constraint by involving field modes at different temperatures, the high temperature ${x}$-polarization and the low-temperature isotropic vacuum. In this case, the rates are no longer balanced resulting in a coherent NESS.

The second important observation apparent from Eq. (\ref{SS_Dyn}) and Fig.~\ref{fig:2} is that the values of excited-state populations in the steady state deviate from those expected in canonical thermodynamic equilibrium
\begin{equation} \label{CanEqn_NoC}
    \rho^\text{(c)}_{aa} = \frac{r}{(3r+\gamma)}
\end{equation}
  The deviation of excited-state populations from the Boltzmann distribution then follows from Eq. (\ref{SS_Dyn})
 \begin{align}
    \rho^{R}_{ab} &= \frac{\Delta \rho_{aa}}{\rho^\text{(c)}_{aa}} \label{CanEqn} \\
    \rho^{I}_{ab} &= -\frac{\Delta}{(r+\gamma)} \rho^{R}_{ab} \label{CanEqn_Imag}
\end{align}
 These expressions are a central result of this work. They establish that  polarized incoherent driving leads to the formation of a coherent non-equilibrium steady-state (NESS) characterized by substantial Fano coherences in the energy eigenstate basis of the V-system.

  Significantly, Eq. (\ref{CanEqn}) suggests that the relative deviation of excited-state populations in the NESS from their values in canonical thermodynamic equilibrium  (\ref{CanEqn_NoC}) is equal to the real part of the Fano coherence.
  In other words, \textit{the real part of the steady-state coherence is directly proportional to the difference in the excited state populations with and without Fano coherence}.

    Equation (\ref{CanEqn})  thus provides a direct connection between steady-state Fano coherences and excited-state populations  of the V-system continuously driven by a polarized incoherent radiation field.
  As such,  Eq.~(\ref{CanEqn}) enables  direct experimental detection of the steady-state Fano coherences through measuring the deviation of excited-state populations  from their canonical equilibrium values (\ref{CanEqn_NoC}), as shown in Sec. IV.  Because it is typically much easier to detect eigenstate populations than coherences, steady-state Fano coherences may be significantly easier to observe experimentally than their transient counterparts \cite{Dodin:18}.

The physical origin of the non-equilibrium coherences (to be further clarified in Sec. IIIA below) can be traced back to Fano interference between the electric dipole transitions induced by the interaction with a common incoherent light field mode.
    This interference is manifested in the population-to-coherence coupling terms in the BR equation (\ref{QME2}), which show that the presence of a positive real part of the coherence $\rho^{R}_{ab}(t)$, suppresses the excited state populations. \par

We now turn to the study of the dependence of steady-state Fano coherences on the dimensionless parameters $\bar{n}$ and $\Delta / \gamma$ that control the dynamics of the incoherently driven V-system in the absence of relaxation and decoherence.
Figure \ref{fig:3}(a) shows the dependence of  steady-state Fano coherences on the average occupation number of thermal photons $\bar{n}=r/\gamma$ in the pumping field. The coherences  increase gradually with the pumping intensity and approach a common limit that does not depend on $\Delta/\gamma$.
As shown in Fig.~\ref{fig:3}(b)  the steady-state coherence are nearly independent of  the excited-state splitting $\Delta/\gamma$ in the weak pumping limit  $\bar{n}\ll 1$. At higher pumping intensities, the coherences begin to decline monotonously with inclreasing $\Delta/\gamma$.

To determine whether the real part of steady-state Fano coherence can reach a maximum as a function of $\Delta/\gamma$ and $\bar{n}$, we calculate the first derivatives of Eq.~(\ref{CanEqn_Imag}) with respect to these parameters
\begin{align}
    \frac{\partial }{\partial \bar{n}}\rho^{R}_{ab} &= \frac{(3\bar{n}^{2}+2\bar{n}+1)(\Delta/\gamma)^{2}+(\bar{n}^{2}+2\bar{n}+1)}{[(3\bar{n}+1)(\Delta/\gamma)^{2}+(4\bar{n}^{2}+5\bar{n}+1)]^{2}} \nonumber \\
    \frac{\partial }{\partial (\Delta/\gamma)}\rho^{R}_{ab} &= -\frac{2\bar{n}(\bar{n}+1)(\Delta/\gamma)}{[(3\bar{n}+1)(\Delta/\gamma)^{2}+(4\bar{n}^{2}+5\bar{n}+1)]^{2}}
\end{align} \par
The derivatives do not vanish for $\bar{n}>0$ and $\Delta/\gamma>0$, and therefore  steady-state Fano coherences do not display maxima or minima. This behavior is illustrated in Fig.~\ref{fig:3}(c), which plots the real part of steady-state Fano coherence as a function of $\bar{n}$ and $\Delta/\gamma$.
The magnitude of the steady-state Fano coherence is therefore maximal at a boundary of the two-dimensional region depicted in Fig.~\ref{fig:3}(c).  More specifically, the maximum is achieved in the small excited-state splitting regime $\Delta/\gamma\ll 1$ regardless of the value of $\bar{n}$. As the pumping rate increases, the region of maximum coherence is shifted to higher values of $\Delta/\gamma$.

As an alternative coherence measure, consider the  ratio \cite{Tscherbul:14,Dodin:16}
\begin{equation}\label{CratioDef}
\mathcal{C} = \frac{\rho_{ab}^R}{\rho_{aa}},
\end{equation}
which quantifies the relative magnitude of  coherences vs. excited-state populations. A substantial value of $\mathcal{C}\simeq 1$ indicates the possibility of a significant coherent contribution to excited-state  dynamics, affecting  the values of observables such as fluorescence emission intensities (see Sec. IV below).  From Eq. (\ref{SS_Dyn}) we obtain
\begin{equation}\label{Cratio1}
\mathcal{C} =  \frac{1}{1+\frac{\Delta^2}{\gamma(r+\gamma)} }
\end{equation}
which is  less than unity as expected from the Cauchy-Swartz inequality, $|\rho_{ab}|^2\leq \rho_{aa}\rho_{bb}$. The ratio (\ref{Cratio1})  tends to unity  for $\frac{\Delta^2}{\gamma(r+\gamma)}\ll 1$, {\it i.e.}, in the regime {\it of small excited-state splitting  $\Delta$ compared to  $\sqrt{\gamma(r+\gamma)}$.} In the weak-pumping limit $(r\ll \gamma)$, this condition simplifies to  ${\Delta} \ll \gamma$. In the  strong-pumping limit ($r\gg  \gamma$),  steady-state Fano coherences are maximized relative to excited-state populations when ${\Delta} \ll \sqrt{r\gamma}$, which is a less restrictive condition than in the weak-pumping limit.

\subsection{Physical origin of steady-state Fano coherence: The two-bath nonequilibrium transport model}

Previous theoretical work has shown that Fano coherences induced in the V-system irradiated by isotropic incoherent radiation are transient and eventually decay back to zero \cite{Agarwal:01, Tscherbul:15, Dodin:16}. In contrast, when the V-system is driven by polarized incoherent radiation, Fano coherences remain non-zero in the steady state, suggesting the presence of a dynamic equilibrium  \cite{Agarwal:01,Dodin:18}.
 In our previous work we suggested an analogy between the latter situation and one of the V-system interacting with two independent thermal baths \cite{Dodin:18}, resulting in non-equilibrium heat transport across the V-system and steady-state coherences associated with it \cite{Segal:00,Manzano:13,Benenti:17}.  Here, we make this analogy more precise by showing that the BR equations of motion for the  V-system  driven by polarized incoherent radiation are equivalent to those describing quantum transport in a system consisting of two coupled two-level systems (qubits). We identify the imaginary part of steady-state Fano coherence with the non-equilibrium flux  across the dimer system. This result unravels a direct connection between the seemingly unrelated phenomena of incoherent driving of multilevel quantum systems and non-equilibrium transport.

Consider a system of two qubits coherently coupled by an exchange or dipolar interaction quantified by the hopping  parameter $t=2\Delta$, as shown in Fig.~\ref{fig:1}(b).  In the weak-pumping limit only the ground $|g\rangle=|g_1g_2\rangle$ and singly excited eigenstates
\begin{align}\notag
|a\rangle&=\frac{1}{\sqrt{2}}(|e_1g_2\rangle+|e_2g_1\rangle), \\
|b\rangle&=\frac{1}{\sqrt{2}}(|e_1g_2\rangle-|e_2g_1\rangle) \label{TLSeigenstates}
\end{align}
of the two-qubit system are appreciably populated, leading to an effective V-system  description \cite{Tscherbul:18,Li:15} illustrated in  Fig.~\ref{fig:1}(a). Here $|g_i\rangle$ and $|e_i\rangle$  stand for the ground and excited computational basis states of the $i$-th  qubit. In addition, each qubit is coupled to a thermal bath maintained at different temperatures $T_L$ and $T_R$ as shown in Fig.~\ref{fig:1}(b). The perturbative BR master equations describing non-equilibrium transport of energy through the two-qubit system are, in the eigenstate basis  of the coupled two-qubit system (\ref{TLSeigenstates})  \cite{Li:15}
\begin{align}
    \Dot{\rho}_{aa} &= 2\Gamma^{+}_{aa}(\varepsilon_{a}) \rho_{gg} - 2\Gamma^{-}_{aa}(\varepsilon_{a}) \rho_{aa} - \Gamma^{-}_{ab}(\varepsilon_{b}) \rho_{ab} - \Gamma^{-}_{ba}(\varepsilon_{b}) \rho_{ba} \nonumber \\
    \Dot{\rho}_{bb} &= 2\Gamma^{+}_{bb}(\varepsilon_{b}) \rho_{gg} - 2\Gamma^{-}_{bb}(\varepsilon_{b}) \rho_{bb} - \Gamma^{-}_{ab}(\varepsilon_{a}) \rho_{ab} - \Gamma^{-}_{ba}(\varepsilon_{a}) \rho_{ba} \nonumber \\
    \Dot{\rho}_{ab} &= \big[\Gamma^{+}_{ba}(\varepsilon_{a}) \rho_{gg} - \Gamma^{-}_{ba}(\varepsilon_{a}) \rho_{aa}\big] +  \big[\Gamma^{+}_{ba}(\varepsilon_{b}) \rho_{gg} - \Gamma^{-}_{ba}(\varepsilon_{b}) \rho_{bb}\big] + i\Delta \rho_{ab} - \big[\Gamma^{-}_{aa}(\varepsilon_{a}) + \Gamma^{-}_{bb}(\varepsilon_{b})\big] \rho_{ab} \label{QME_Sun}
\end{align}
Significantly,  these equations describe the setup, where qubit 1 is  coupled {\it only} to the left bath and qubit 2 {\it only} to the right bath, as can be shown by recasting the system-bath coupling given by Eq. (A.1) of Ref. \cite{Li:15} in the site basis via Eq. (\ref{TLSeigenstates}).
In Eq. (\ref{QME_Sun}), $\varepsilon_{i} = E_{i} - E_{g}$ is the energy difference between the excited state $i = \ket{a},\enspace \ket{b}$ and the ground state $\ket{g}$, $\Delta = E_{a} - E_{b}$ is the excited state splitting and the dissipation rates $\Gamma^{\pm}_{ij}(\omega)$ are  given by
\begin{align}
    \Gamma^{-}_{ij}(\omega) &= \frac{1}{2} \gamma^{(L)}_{ij}(\omega) \big[\bar{n}_{L}(\omega)+1 \big] + \frac{1}{2} \gamma^{(R)}_{ij}(\omega) \big[\bar{n}_{R}(\omega)+1 \big] \nonumber \\
    \Gamma^{+}_{ij}(\omega) &= \frac{1}{2} \gamma^{(L)}_{ij}(\omega) \bar{n}_{L}(\omega) + \frac{1}{2} \gamma^{(R)}_{ij}(\omega) \bar{n}_{R} \label{QME_Sun2},
\end{align}
$\bar{n}_{\alpha} = (e^{\hbar\omega/T_{\alpha}}-1)^{-1}$  is the average number of photons in the  left and right baths $\alpha=L,R$, and  $\gamma^{\alpha}_{ij}(\omega)$ are the coupling spectra of the $\alpha$-th bath
\begin{equation}
    \gamma^{\alpha}_{ij}(\omega) = 2\pi \sum_{k_{\alpha}} g^{*}_{i,k_{\alpha}} g_{j,k_{\alpha}} \delta(\omega-\omega_{k_{\alpha}})= [\gamma^{\alpha}_{ji}(\omega)]^{*}
\end{equation}
where $g_{i, k_{\alpha}} = \sqrt{\frac{\hslash \omega_{k_{\alpha}}}{2 \epsilon_{0} V}} \big(\bm{\mu}_{ij} \cdot \bm{\varepsilon}_{k_{\alpha} \lambda} \big)$ is the light-matter coupling coefficient. The cross specta $\gamma^{\alpha}_{ij}$ ($i \neq j$)  quantify the interference between the transitions $\ket{a} \rightarrow \ket{g}$ and $\ket{b} \rightarrow \ket{g}$   \cite{Li:15}
\begin{equation}\label{weight_factors}
    |\gamma^{\alpha}_{ij}(\omega)|^{2} = f_{\alpha}(\omega)  \gamma^{\alpha}_{ii}(\omega) \gamma^{\alpha}_{jj}(\omega),
\end{equation}
where the weight factors $f_{\alpha}$ (assumed henceforth to be frequency independent) are determined by  the form of the system-bath coupling \cite{Li:15}. In the case of incoherent light-matter coupling of interest here, the weight factors are directly related to the transition dipole alignment parameters $p_{ij}$ \cite{Tscherbul:15}.

We suggest that the V-system irradiated by polarized incoherent radiation can be thought of as a system of two qubits interacting with each other and with two independent thermal baths, as shown in Fig.~\ref{fig:1}(b). A hot bath with $T_L=5800$~K is responsible for incoherent pumping of the qubit coupled to it, which allows us to set $\bar{n}_{L} = \bar{n}$  in Eq. (\ref{QME_Sun}).   A cold bath with $T_R=0$ accounts for spontaneous emission due to the coupling of the second qubit to the vacuum modes of the electromagnetic field, and hence we can set $\bar{n}_{R}=0$ in Eq. (\ref{QME_Sun}).
With these simplifications, Eqs. (\ref{QME_Sun}) and (\ref{QME_Sun2}) reduce to
\small
\begin{align}
    \Dot{\rho}_{aa} &= r_{aa}^{L} \rho_{gg} - (r_{aa}^L+{\gamma}_{aa}^L + {\gamma}_{aa}^R) \rho_{aa} - \frac{1}{2} \sqrt{f_{L}}\big(\sqrt{r_{aa}^Lr_{bb}^L}+\sqrt{{\gamma}_{aa}^L{\gamma}_{bb}^L}\big) (\rho_{ab}+\rho_{ba}) - \frac{1}{2} \sqrt{f_{R}} \sqrt{{\gamma}^R_{aa}{\gamma}^R_{bb}} (\rho_{ab}+\rho_{ba}) \nonumber \\
        \Dot{\rho}_{bb} &= r_{bb}^{L} \rho_{gg} - (r_{bb}^L+{\gamma}_{bb}^L + {\gamma}_{bb}^R) \rho_{bb} - \frac{1}{2} \sqrt{f_{L}}\big(\sqrt{r_{aa}^Lr_{bb}^L}+\sqrt{{\gamma}_{aa}^L{\gamma}_{bb}^L}\big) (\rho_{ab}+\rho_{ba}) - \frac{1}{2} \sqrt{f_{R}} \sqrt{{\gamma}^R_{aa}{\gamma}^R_{bb}} (\rho_{ab}+\rho_{ba}) \nonumber \\

\begin{split}
    \Dot{\rho}_{ab} &= \sqrt{f_{L}} \sqrt{r_{aa}^Lr_{bb}^L} \rho_{gg} - \frac{1}{2} \sqrt{f_{L}}\big(\sqrt{r_{aa}^Lr_{bb}^L}+\sqrt{{\gamma}^L_{aa}{\gamma}_{bb}^L}\big) (\rho_{aa}+\rho_{bb}) - \frac{1}{2} \sqrt{f_{R}} \sqrt{{\gamma}^R_{aa}{\gamma}^R_{bb}} (\rho_{aa}+\rho_{bb}) - i\Delta \rho_{ab} \\ &\qquad - \frac{1}{2} (r_{aa}^L+r_{bb}^L+{\gamma}^L_{aa}+{\gamma}_{bb}^L+{\gamma}_{aa}^R+{\gamma}^R_{bb}) \rho_{ab},
\end{split} \label{BR_Transport_Eqn}
\end{align}\normalsize
where we use the same incoherent pumping and spontaneous decay parameters $\gamma^{\alpha}_{ij}$ and $r^{\alpha}_{ij}$ ($ i = a, b$;  $\alpha = L, R$) as the transport model equations (\ref{QME_Sun}) and (\ref{QME_Sun2}) \cite{Li:15}.
The  incoherent pumping rates due to the left (hot) bath are given by $r_{ii}^L = \bar{n}_L {\gamma}^L_{ii}$, where ${\gamma}^L_{ii}$ are the corresponding spontaneous decay rates. The right (cold) bath can only induce spontaneous decay, whose rates are given by  ${\gamma}^R_{ii}$.

In this paper, we consider the V-system with orthogonal transition dipole moments (such as the Ca atom in Sec.~IV  irradiated by polarized incoherent radiation.  Because of the orthogonality condition, there is no interference in spontaneous emission  \cite{Dodin:18} and we can thus set $f_{\alpha}= 0$ for spontaneous emission terms in Eq. (\ref{BR_Transport_Eqn}).  In contrast, we have $f_{\alpha} = 1$  for polarized incoherent driving \cite{Dodin:18}. As a result, Eq. ~(\ref{BR_Transport_Eqn}) can be recast in the form
\begin{align}
    \Dot{\rho}_{aa} &= r_{aa}^{L} \rho_{gg} - (r_{aa}^L+{\gamma}_{aa}^L + {\gamma}_{aa}^R) \rho_{aa} - \frac{1}{2} \sqrt{r_{aa}^Lr_{bb}^L}(\rho_{ab}+\rho_{ba})  \nonumber \\
        \Dot{\rho}_{bb} &= r_{bb}^{L} \rho_{gg} - (r_{bb}^L+{\gamma}_{bb}^L + {\gamma}_{bb}^R) \rho_{bb} - \frac{1}{2}   \sqrt{r_{aa}^Lr_{bb}^L} (\rho_{ab}+\rho_{ba}) \nonumber \\
    \Dot{\rho}_{ab} &= \sqrt{r_{aa}^Lr_{bb}^L} \rho_{gg} - \frac{1}{2}  \sqrt{r_{aa}^Lr_{bb}^L} (\rho_{aa}+\rho_{bb}) - i\Delta \rho_{ab}  - \frac{1}{2} (r_{aa}^L+r_{bb}^L+{\gamma}^L_{aa}+{\gamma}_{bb}^L+{\gamma}_{aa}^R+{\gamma}^R_{bb}) \rho_{ab}
\label{BR_Transport_Eqn_set_factors}
\end{align}\normalsize

These equations are identical to the BR quantum optical master equation (\ref{QME1}), with $\gamma_{i} = {\gamma}_{ii}^L + {\gamma}^R_{ii}$ and $r_i=r_{ii}^L=\bar{n}_L\gamma^L_{ii}$,  thus establishing equivalence between the V-system driven by polarized incoherent light and a qubit dimer coupled to two independent baths.
Significantly, the transport model gives the ratio of incoherent driving and spontaneous decay rates ${r_i}/\gamma_i=r_{ii}^L/(\gamma_{ii}^L + \gamma_{ii}^R)$ at odds with the equilibrium fluctuation-dissipation theorem, based on which one would expect ${r_i}/\gamma_i = r_{ii}^L/\gamma_{ii}^L=\bar{n}_L$. As discussed above and in Refs.~\cite{Agarwal:01,Dodin:19}, it is this  imbalance between incoherent driving and spontaneous decay   that leads to   the formation of coherent NESS.

To characterize non-equilibrium transport in our model two-qubit system, we calculate the energy flux from the ``hot'' qubit 1 to the ``cold'' qubit 2 \cite{Manzano:13,Li:15}
\begin{equation}
J_{1-2} = -i \langle [\hat{\sigma}^{z}_{1}, \hat{H}_{s}] \rangle =
         -i 2g \text{Tr} \big[ \rho \big(\ket{a} \bra{b} - \ket{b} \bra{a}\big)\big] = 4g \textrm{Im}\{\langle a|\rho | b \rangle \},\label{J1_to_2}
\end{equation}
where $\hat{H}_{s} = \frac{1}{2} \omega_{1}\hat{\sigma}^{z}_{1} + \frac{1}{2} \omega_{2}\hat{\sigma}^{z}_{2} + g (\hat{\sigma}^{+}_{1}\hat{\sigma}^{-}_{2} + \hat{\sigma}^{-}_{1}\hat{\sigma}^{+}_{2})$ is the  Hamiltonian of the  two-qubit system expressed via the jump operators $\hat{\sigma}_i^\pm$ which are defined as $\hat{\sigma}_i^{-} = \ket{g_{i}} \bra{e_{i}}$, $\hat{\sigma}_i^{+} = \ket{e_{i}} \bra{g_{i}}$, $\hat{\sigma}_i^{z} = \ket{e_{i}} \bra{e_{i}} - \ket{g_{i}} \bra{g_{i}}$. Here, $\ket{e_{i}}$, $\ket{g_{i}}; \enspace i = 1,2$ are the excited and ground states of the  coupled qubits 1 and 2 in the site basis, $g$ is the qubit-bath coupling, and the trace is taken over the bath degrees of freedom.

Equation (\ref{J1_to_2}) establishes that the energy flux  from  qubit 1 to qubit 2 is proportional to the  imaginary part of Fano coherence in the energy eigenstate basis (\ref{TLSeigenstates}) of the dimer. This clarifies the physical significance of steady-state Fano coherences as being responsible for radiative energy transfer from sunlight-driven qubit 1 to qubit 2 that is  coupled to the vacuum modes of the electromagnetic field. In addition, the real part of coherence in the energy eigenstate basis is proportional to the difference of excited state populations in the site basis \cite{Tscherbul:18}.

\subsection{Effect of excited-state relaxation and decoherence}

Realistic quantum systems are always subject to environmental perturbations causing relaxation and decoherence. In this section, we explore the robustness of steady-state Fano coherences against these detrimental effects. To this end, we follow previous theoretical work \cite{Rebentrost:09,Chin:09,Tscherbul:18} and introduce phenomenological relaxation and decoherence channels represented by the terms $\Gamma \rho_{aa}$ and $\gamma_d\rho_{ab}$ in Eq. (\ref{QME2}).
Following the analysis presented above, we obtain steady state solutions as a function of relaxation and decoherence rates $\Gamma$ and $\gamma_d$:
\begin{align} \label{Dyn_Dec_Rel}
    \rho_{aa} &= \frac{r [\Delta^{2}+(\gamma + \gamma_{d})(r+\gamma+\gamma_{d})]} {(3r+\gamma+\Gamma)[\Delta^{2}+(r+\gamma+\gamma_{d})^{2}]-3r^{2}(r+\gamma+\gamma_{d})} \nonumber \\
    \rho^{R}_{ab} &= \frac{r (\gamma+\Gamma) (r+\gamma+\gamma_{d})}{(3r+\gamma+\Gamma)[\Delta^{2}+(r+\gamma+\gamma_{d})^{2}]-3r^{2}(r+\gamma+\gamma_{d})} \nonumber \\
    \rho^{I}_{ab} &= -\frac{\Delta}{(r+\gamma+\gamma_{d})} \rho^{R}_{ab}
\end{align} \par
These equations suggest that both the real and imaginary steady state coherences can survive in the presence of relaxation and decoherence. Increasing the relaxation rate does not significantly affect the steady-state coherence in the typical limit  $\Gamma \gg r+\gamma$, where the dependence $\rho^{R}_{ab}(\Gamma) \simeq \frac{\gamma+\Gamma}{3r+\gamma+\Gamma}$ is weak (Ref.~\cite{KoyuThesis:19} considers the effect of relaxation is more detail). We therefore focus on the case of pure decoherence (or dephasing) assuming $\Gamma=0$.

In Fig.~\ref{fig:4} we plot the dependence of the steady-state Fano coherence on the excited-state splitting and the reduced decoherence rate $\gamma_d/\gamma$  (\ref{Dyn_Dec_Rel}).  We observe that, regardless of the pumping intensity, the steady-state coherences are maximized for small excited-state splittings $\Delta/\gamma \ll 1$. In the weak pumping limit illustrated in Fig.~\ref{fig:4}(a) the coherences also decrease rapidly with the decoherence rate, falling below one part in $10^{3}$ for $\gamma_d/\gamma > 6$. Similar trends are observed in the case of intermediate pumping ($\bar{n}=1$), even though the absolute magnitude of the steady-state coherence in this regime is larger by two orders of magnitude.  The coherences in the strong pumping limit ($\bar{n}\gg 1$) are large and while they they do not fall off as strongly with $\Delta/\gamma$ they do get significantly suppressed  by decoherence. The extent of this suppression appears insensitive to the pumping rate.

Remarkably, as shown in Figs.~\ref{fig:4}(a)-(c),  the presence  of decoherence can {\it enhance} the magnitude of steady-state Fano coherences.  For instance, at $\Delta/\gamma_d=2$ the value of $\rho_{ab}^{R}$ passes through a maximum near $\gamma_d=2$ and then decreases again at higher $\gamma_d$.  This enhancement  is particularly pronounced for large $\Delta/\gamma$ in the weak-pumping limit, where we observe up to 5-fold coherence enhancements  \cite{KoyuThesis:19}.   To further explore this counterintuitive effect, we rewrite Eq.~(\ref{Dyn_Dec_Rel}) in terms of the dimensionless parameters  $\Tilde{\gamma}_{d} = \gamma_{d}/\gamma$ and $\Tilde{\Delta} = \Delta/\gamma$
\begin{equation} \label{SS_Real}
    \rho^{R}_{ab} = \frac{\bar{n} (\bar{n}+1+\Tilde{\gamma}_{d})}{(3\bar{n}+1)[\Tilde{\Delta}^{2}+(\bar{n}+1+\Tilde{\gamma}_{d})^{2}]-3\bar{n}^{2}(\bar{n}+1+\Tilde{\gamma}_{d})}
\end{equation}
The roots of the equation $ \frac{d}{d\Tilde{\gamma}_{d}}\rho_{ab}^{R}=0$  are given by  $\Tilde{\gamma}_{d} = \pm \tilde{\Delta}  -\bar{n} - 1$   \cite{KoyuThesis:19}. Picking the physical root corresponding to $\tilde{\Delta}>0$, we obtain the optimal decoherence rate
\begin{equation}\label{gammadRoot}
  \gamma_{d} =  {\Delta}  -{r} - \gamma
  \end{equation}
  that maximizes the value of the steady-state Fano coherence.
In the weak pumping regime, Eq.~(\ref{gammadRoot})  simplifies to  ${\gamma}_{d} \approx {\Delta}$ which defines the diagonal  ``line of optimal decoherence'' in Figs.~\ref{fig:4}(a) and (b), along which the steady-state Fano coherence takes a maximum value. Importantly, the maximum of  the steady-state Fano coherence as a function of $\gamma_d$ only appears when the optimal decoherence rate in Eq. (\ref{gammadRoot}) is positive (${\Delta}\ge r+\gamma$), which  corresponds to the underdamped regime of V-system dynamics \cite{Koyu:18,Tscherbul:14,Dodin:16,Dodin:18}.
This is illustrated in Fig.~\ref{fig:4}(c), which shows that the maximum of $\rho_{ab}^R$ is located along the vertical line  of constant $\gamma_d/\gamma=10$.

The population-to-coherence ratio (\ref{CratioDef}) in the presence of dephasing can be obtained from Eq. (\ref{Dyn_Dec_Rel})
\begin{equation}
\mathcal{C} = \frac{1}{1+ \frac{\gamma_d}{\gamma} + \frac{\Delta^2}{\gamma(r+\gamma+\gamma_d)} }.
\end{equation}
The ratio takes the maximum value $\mathcal{C}_\text{max}=\frac{1}{1+\gamma_d/\gamma + (r+\gamma+\gamma_d)/\gamma }$ when the sum in the denominator
is a minimum, which occurs when $\gamma_d=\Delta-r-\gamma$. This is the same condition as required for the maximization of the real part of steady-state Fano coherence (\ref{gammadRoot}).

 Under typical molecular excitation  conditions, nonradiative dephasing is fast compared with radiative processes ($\gamma_d\gg \gamma, r$)  and we obtain $\mathcal{C} \simeq \frac{1}{1+\gamma_d/\gamma + \Delta^2/(\gamma\gamma_d) }\ll 1$. In the limit of small $\Delta\ll \sqrt{\gamma\gamma_d}$ the last term in the denominator can be neglected, giving
  $\mathcal{C} \simeq \frac{1}{1+\gamma_d/\gamma }\simeq \gamma/\gamma_d \ll 1$.
   Thus, {\it  the ratio of steady-state Fano coherences to excited-state populations will be suppressed by the factor $\gamma_d/\gamma$ in the presence of environmental dephasing, as long as the system-environment coupling responsible for the dephasing does not generate any steady-state coherence} (as assumed here, see Sec. III).

Figure~\ref{fig:Cratio} shows the steady-state coherence-to-population ratio as a function of dephasing. In accordance with  the analytic result obtained above (\ref{gammadRoot}), we observe the emergence of a maximum at the optimal decoherence rate $\gamma_d=\Delta-r-\gamma$. The maximum is only present at sufficiently large excited-state splittings $\Delta$ such that $\Delta-r-\gamma > 0$ (underdamped regime of V-system dynamics  \cite{Tscherbul:14,Dodin:16a,Koyu:18}) as shown in Figs.~\ref{fig:Cratio}(a) and (b).   Decreasing the value of $\Delta$ brings the V-system into the overdamped regime \cite{Tscherbul:14,Dodin:16a,Koyu:18} characterized by $\Delta/\gamma<1$. As shown in Figs.~\ref{fig:Cratio}(c) and (d), this leads to the disappearance of the maximum and the  expected monotonic decrease of  the $\mathcal{C}$-ratio with increasing  decoherence rate.

While the ability of dephasing to enhance steady-state coherence in the  underdamped regime is surprising, the dephasing enhanced steady-state coherence can be understood by considering the individual contributing excitations.
In the underdamped regime, one mechanism of coherence loss arises due to the cancellation of excitations at different times that carry different phases due to their unitary evolution in the excited state manifold [see Fig~\ref{fig:timescales_dephasing}(b)]. By introducing an explicit dephasing channel, excitations generated at earlier times lose more coherences than those generated later. As  a result, these excitations do not destructively interfere  as much as they could in the absence of dephasing. The dephasing then weights the phase average towards a narrower window of excitation times, decreasing the ensemble-induced dephasing process. However, dephasing leads to coherence loss at the level of individual excitations.
Consequently, this trade-off leads to a competition between the two effects of increased dephasing, allowing for dephasing-enhanced steady state coherences in certain regimes when the decreased ensemble dephasing outweighs the increased excitation level dephasing.

We conclude that in the underdamped (or large-$\Delta$) regime of V-system dynamics, steady-state  Fano coherence are maximized when the decoherence rate is equal to the energy splitting between the excited states.  The physical origin of the maximization can be interpreted at the level of individual incoherent excitations, whose unitary evolution is accompanied by environmental decoherence. The competition of these mechanisms can result in an enhancement of steady-state coherence through minimization of destructive interference caused by coherent evolution. A similar mechanism is at play in environment-assisted quantum transport, whereby the addition of a moderate amount of noise positively affects the energy flux in  multichromophoric  reaction complexes \cite{Manzano:13,Wu:10,Rebentrost:09,Chin:09}.
 The decoherence-induced enhancement of Fano coherences could be used to facilitate their  experimental observation via measuring excited-state populations, as discussed in the following section.

\section{Experimental detection of steady-state Fano coherence }

In our previous work \cite{Dodin:18}, we proposed a scheme for the experimental observation of  {\it transient} Fano coherences by detecting  the fluorescence signal emitted by incoherently pumped Calcium atoms. This scheme suffers from two  difficulties: First, the transient nature of noise-induced coherent dynamics makes it sensitive to the turn-on time of the radiation. In particular, Fano coherences are known to vanish in the limit where the turn-on time is much longer than that of spontaneous emission \cite{Dodin:16a}.
Second, because the total fluorescence intensity is independent of Fano coherence \cite{Dodin:18}, it required the detection of the fluorescence emitted into a specific range of solid angles.

In this section, we eliminate these difficulties by arguing that steady-state Fano coherences  can be observed by measuring the {\it total steady-state} fluorescence signal emitted by Calcium atoms irradiated by polarized vs. isotropic incoherent light.  Unlike the method proposed in Ref. \cite{Dodin:18}, the new detection scheme  requires neither rapid  turn-on of the radiation field nor spatially resolved detection of the fluorescence signal.

 Our proposed experimental setup is similar to that described in our previous work (see Fig.~\ref{fig:1}(a) and Fig. 1 of Ref.~\cite{Dodin:18}) and consists of a beam of Ca atoms initially prepared in the ground $^1$S$_0$ electronic state. The atoms are continuously  irradiated with spectrally broadened light polarized in the $x$-direction,  inducing the electric dipole transition $^1$S$_0\to {^1}\textrm{P}_{m_J}$ from the $J=0$ ground state to $J=1$ excited states with $m_J=\pm 1$. The excited states are split by an external magnetic field pointing in the $z$-direction, forming  a nearly perfect V-system with tunable excited-state splitting $\Delta$ \cite{Dodin:18}. Following initial turn-on of incoherent excitation, a fraction of Ca atoms in the beam will be excited to the $^1\textrm{P}_{m_J}$ states. The excited atoms will decay to the ground state emitting fluorescence photons.

 The average intensity of the radiation emitted by Ca atoms in the direction  $(\theta, \phi)$ at a distance $R$ away from the source is \cite{Dodin:18}
\begin{equation} \label{Int_Eq}
    \langle I(\mathbf{R},t) \rangle = \frac{n_{r}\omega^{4}_{0}}{32\pi^{2}
    \epsilon_{0} c^{3} R^{2}} \bigg[ \frac{1+\text{cos}^{2}\theta}{2} \big(\rho_{aa}(t') + \rho_{bb}(t')\big) + \text{sin}^{2}\theta \big(\text{cos}2\phi \rho^{R}_{ab}(t')-\text{sin}2\phi \rho^{R}_{ab}(t') \big) \bigg]
 \end{equation}
 where  $t' = t + R/c$ is the retarded time, $n_{r}$ is the refractive index of the medium, $\textit{c}$ is the speed of light in free space. Integrating Eq.~(\ref{Int_Eq}) over all spatial directions ($\theta, \phi$) we obtain the total emitted intensity $I = \frac{8\pi}{3} I^{0} (\rho_{aa} + \rho_{bb})$, where $I^{0} = n_{r}\omega^{4}_{0}/(32\pi^{2}\epsilon_{0} c^{3} R^{2})$.
For a symmetric V-system $\rho_{aa}=\rho_{bb}$, this expression  further simplifies to
\begin{equation} \label{I_final2}
    I = \frac{16\pi}{3} I^{0} \rho_{aa}
\end{equation}
Importantly, unlike its spatially resolved counterpart (\ref{Int_Eq}) the integrated fluorescence intensity depends only on the excited state population and not on the Fano coherence. Therefore, in order to directly observe transient Fano coherences,  it is necessary to measure the intensity emitted into specific domains of space \cite{Dodin:18} in such a way that the partially integrated  fluorescence intensity is made to explicitly depend of Fano coherence terms $\rho_{ab}$.

Here, we show that it is not necessary to implement spatially resolved fluorescence detection  \cite{Dodin:18} to observe steady-state Fano coherences in a V-system excited by polarized incoherent light.
As shown in Sec. III above, the magnitude of the real part of steady-state Fano coherence is directly related to the {\it deviation of excited-state populations from their values in thermodynamic equilibrium} via Eq.~(\ref{CanEqn_Imag}).
As such, observing  these deviations could be used to directly probe steady-state Fano coherences.

More specifically, let the intensity of the emitted light in the absence of Fano coherence be $I^{(0)}$. This intensity  corresponds to the excited-state population in the absence of Fano coherence given by Eq.~(\ref{CanEqn_NoC}). From Eqs.~(\ref{CanEqn}) and (\ref{I_final2}), the relative difference of the emitted light intensity with and without steady-state Fano coherence is
\begin{equation}\label{DeltaI}
    \frac{\Delta I}{I^{0}} = \frac{\Delta \rho_{aa}}{\rho_{aa}^{(c)}} = \rho^{R}_{ab}
\end{equation}
We see that in the coherent NESS induced by $x$-polarized incoherent driving of the Calcium V-system,  excited-state populations are suppressed compared to the canonical Boltzmann distribution. The intensity of the light emitted by the Calcium atoms  driven into the NESS is therefore diminished compared to the intensity that would be emitted by the atoms in coherence-free canonical thermal equilibrium (attainable by isotropic incoherent driving \cite{Tscherbul:14,Dodin:16,Dodin:18}). The relative difference in the fluorescence signals emitted by the atoms driven by $x$-polarized vs. isotropic incoherent light can therefore be interpreted as an experimental signature of   steady-state Fano coherences.

Figure~\ref{fig:5} shows the experimentally relevant fluorescence difference signals calculated by numerical integration of the BR equations. We observe rich transient dynamics, after which the signals reach their non-equilibrium steady-state values consistent with Eq. (\ref{DeltaI}). The observable relative intensity difference remains fairly small ($<1\%$) in the weak-pumping limit  but grows significantly with the pumping intensity, reaching $23\%$ for $\bar{n}=10^3$ and $\Delta/\gamma=10$. As pointed out in Sec. IIIB above, it might be possible to further enhance the  steady-state Fano coherence (and hence the fluorescence difference signal) by inducing moderate decoherence between the excited states of the calcium atoms. This could be achieved experimentally by, {\it e.g}, adding magnetic field noise or isolating the atoms in a rare-gas host matrix \cite{Andrews:78,Upadhuay:19}.

\section{Summary and conclusions}

We have presented closed-form analytical solutions to  the BR quantum master equations for a three-level V-system driven by polarized incoherent radiation, which reveal the presence of NESS featuring substantial  Fano coherences in the energy eigenstate basis. As pointed out in \cite{Agarwal:01}, the coherent NESS emerge as a result of an imbalance between polarized incoherent excitation and spontaneous emission. The imbalance occurs due to the directional nature of polarized incoherent pumping \cite{Dodin:18}, whereby only a single polarization mode of the radiation field interacts with the V-system \cite{Dodin:19}. As a result, polarized absorption rates are smaller by a factor of 4 that their isotropic counterparts \cite{Dodin:18} while the rates of spontaneous emission remain the same as in the case of unpolarized (isotropic) incoherent pumping, where both polarization modes participate in the emission process. The rates of isotropic incoherent pumping $r$ and spontaneous emission $\gamma$ are balanced, {\it i.e.} related by the equilibrium fluctuation-dissipation theorem $r=\bar{n}\gamma$, and thus no steady-state Fano coherences survive in the V-system driven by unpolarized incoherent light \cite{Agarwal:01}.

The imbalance  between absorption and spontaneous emission that leads to the emergence of steady-state Fano coherences can be thought of as originating from an additional, symmetry-breaking bath, leading to a formal analogy between the V-system driven by polarized incoherent light and a non-equilibrium transport problem involving a system of two qubits coupled to two thermal baths, one at $T=5800$~K responsible for incoherent solar excitation [see  Fig.~\ref{fig:1}(b)] and the other at zero temperature representing spontaneous emission.   We show that in this two-bath model,    the imaginary part of the coherence between the quasi-degenerate excited states in the V-system has a special significance: it is proportional to the non-equilibrium flux between the two-level systems coupled to hot and cold baths.

Our steady-state analysis demonstrates a remarkable relation between steady-state  Fano coherences  and the deviation of excited-state populations from thermal equilibrium: $\Delta \rho_{aa}/\rho^{(c)}_{aa} = \rho^{R}_{ab}$. This relation suggests that signatures of steady-state Fano coherences could be observed through measuring excited-state populations. We further extend our steady-state analysis to include environmental decoherence and relaxation effects, finding that  steady-state Fano coherence persists in the V-system illuminated by polarized incoherent radiation even in the presence of decoherence and relaxation effects.

While  steady-state Fano coherences are generally suppressed by environmental relaxation and decoherence (see Sec. IIIB), we find that the effect of  decoherence can be more subtle.
 In particular,  the real part of the steady-state Fano coherence can be enhanced by a moderate amount of excited-state decoherence, as shown in Fig.~\ref{fig:4}.   The magnitude of the steady-state Fano coherence is maximized when the decoherence rate is equal to the excited energy splitting minus the combined rates of radiative pumping and spontaneous decay ($\gamma_{d}=\Delta-r-\gamma$). We suggest that this counterintuitive enhancement of steady-state Fano coherence occurs due to a suppression of destructive interference of incoherent excitations generated at different times.

Finally, we offer an improved method for the detection of steady-state Fano coherences using Calcium atoms irradiated by polarized incoherent light. Specifically, we propose to detect the signatures of Fano coherences by measuring the deviations of excited-state populations in the NESS from their equilibrium values (obtained by pumping the atoms with isotropic incoherent light). Unlike the scheme proposed in our previous work  \cite{Dodin:18}, this detection scenario  only relies on the total fluorescence intensity measurements, and requires neither spatially resolved fluorescence detection nor rapid turn-on of the incoherent light.

\section*{Acknowledgements} P. B. acknowledges support from the U. S. Air Force office of Scientific Research  (AFOSR) under contract No. FA9550-17-1-0310. We thank Profs. Amar Vutha and Jonathan Weinstein  for stimulating discussions.

\newpage

\begin{figure}[t!]
\captionsetup{singlelinecheck = false, format= hang, justification=raggedright, font=footnotesize, labelsep=space}
\centering
\includegraphics[width=0.9\textwidth]{Fig1}
\caption{(a) Energy level diagram of the V-system composed of a single ground state $g$ and two nearly degenerate excited levels $a$ and $b$. In our proposed experimental realization of the V-system, the ground state corresponds to the  $^1$S$_0$ level of atomic Ca and  the excited states corresponds to the  $^1$P$_1$ levels of  atomic Ca with the total electron orbital angular momentum $J=1$ and its projection $m_J=\pm 1$ on the magnetic field axis. The  excited-state energy splitting  $\Delta$ is continuously tunable with an external magnetic field. The rates of spontaneous decay $\gamma_i$ ($i = a,b$), and those of incoherent pumping  $r_i=\gamma_i \bar{n}$.  (b) An alternative representation of the V-system driven by polarized incoherent light as a pair of coherently coupled qubits interacting with two independent thermal baths at different temperatures.}
\label{fig:1}
\end{figure}

\begin{figure}[t!]
\captionsetup{singlelinecheck = false, format= hang, justification=raggedright, font=footnotesize, labelsep=space}
\centering
\includegraphics[width=0.95\textwidth]{Fig2}
\caption{Time evolution of  excited-state populations and Fano coherences in the V-system weakly (a)-(b) and strongly  (c)-(d) driven by $x$-polarized incoherent light.  (a) Overdamped regime with $\bar{n}=10^{-3}$ and $\Delta/\gamma= 10^{-1}$ (b) Underdamped regime with $\bar{n}=10^{-3}$ and $\Delta/\gamma= 10$;  (c)  $\bar{n}=10^{3}$ and $\Delta/\gamma= 10^{2}$, and (d) $\bar{n}=10^{2}$ and $\Delta/\gamma=2 \times 10^{2}$. The steady-state values of Fano coherences are shown by horizontal dashed lines.}
\label{fig:2}
\end{figure}

\begin{figure}[t!]
\captionsetup{singlelinecheck = false, format= hang, justification=raggedright, font=footnotesize, labelsep=space}
\centering
\includegraphics[width=0.85\textwidth, trim = 0 270 0 260 ]{Fig4}
\caption{Schematic depiction of the unitary time evolution and decay of a single incoherent excitation (a) and of an ensemble of incoherent excitations (b).}
\label{fig:timescales_dephasing}
\end{figure}

\begin{figure}[t!]
\captionsetup{singlelinecheck = false, format= hang, justification=raggedright, font=footnotesize, labelsep=space}
\centering
\includegraphics[width=1.05\textwidth]{Fig3}
\caption{(a) Steady-state Fano coherence plotted as a function of the average number of thermal photons $\bar{n}$ at fixed values of the excited-state splitting $\Delta/\gamma$.  (b) Same as in panel (a) plotted vs $\Delta/\gamma$ at fixed values of  $\bar{n}$ corresponding to the weak, intermediate, and strong pumping regimes.  (c) Two-dimensional contour plot of steady-state Fano coherence as a function of $\Delta/\gamma$ and $\bar{n}$.}
\label{fig:3}
\end{figure}

\begin{figure}[t!]
\captionsetup{singlelinecheck = false, format= hang, justification=raggedright, font=footnotesize, labelsep=space}
\centering
\includegraphics[width=1.05\textwidth]{Fig5}
\caption{Contour plots of steady-state Fano coherence as a function of the excited-state splitting $\Delta/\gamma$ and of the decoherence rate $\gamma_d/\gamma$ under weak (a) and strong (b) $x$-polarized incoherent pumping. The values of the average photon number used are $\bar{n}=0.01$ (a)  and $\bar{n}=100$ (c).  Panel (c) shows the steady-state Fano coherence as a function the decoherence rate and $\bar{n}$ at a fixed $\Delta/\gamma=10$. }
\label{fig:4}
\end{figure}

\begin{figure}[t!]
\captionsetup{singlelinecheck = false, format= hang, justification=raggedright, font=footnotesize, labelsep=space}
\centering
\includegraphics[width=0.85\textwidth]{Fig6}
\caption{Steady-state coherence-to-population  ratio $\mathcal{C}$ plotted as a function of dimensionless decoherence rate  $\gamma_d/\gamma$ in the weak-pumping limit [(a), (c)] and  in the strong-pumping limit [(b), (d)].  The values of  the $\Delta/\gamma$ are  indicated in each panel.  }
\label{fig:Cratio}
\end{figure}

\begin{figure}[t!]
\captionsetup{singlelinecheck = false, format= hang, justification=raggedright, font=footnotesize, labelsep=space}
\centering
\includegraphics[width=0.8\textwidth]{Fig7}
\caption{(a) The ratio of fluorescence intensities calculated for Ca atoms driven by $x$-polarized vs. isotropic incoherent light  in different regimes: (a) $\bar{n}=10^{-2}$ and $\Delta/\gamma= 10^{-1}$; (b) $\bar{n}=10^{-2}$ and $\Delta/\gamma= 10$; (c) $\bar{n}=10^{3}$ and $\Delta/\gamma= 10$;  (d) $\bar{n}=10$ and $\Delta/\gamma= 10^{2}$ .}
\label{fig:5}
\end{figure}

redpajama_set_name: RedPajamaArXiv


text:
Mad Animals (Italian:Animali pazzi) is a 1939 Italian "white-telephones" comedy film directed by Carlo Ludovico Bragaglia and starring Totò, Luisa Ferida and Calisto Bertramo. It was made at the Titanus Studios in Rome.

Plot
Baron Tolomeo dei Tolemei is about to receive the inheritance of a relative, just died. The legacy, however, as he wants the will, must go in part to finance a medical structure for crazy animals. Only then Baron Tolomeo may have the rich heritage. The affair proves complicated, because Tolomeo has a love affair with the beautiful Maria Luisa. The troubles continue when in life of Tolomeo breaks his poor twin-brother Antonio, physically like him, who secretly falls in love with Maria Luisa.

Cast
 Totò as Barone Tolomeo dei Tolomei/His brother
 Luisa Ferida as Maria Luisa
 Calisto Bertramo as Fabrizio, il maggiordomo
 Lilia Dale as Ninetta
 Dina Perbellini as La direttrice dell'ospedale degli animali
 Bianca Stagno Bellincioni as Zia Elisa
 Claudio Ermelli as Il notaio
 Raffaele Giachini as Il pretendente
 Cesare Polacco as Il creditore
 Pina Gallini as La proprietaria del cavallo pazzo

References

Bibliography
 Moliterno, Gino. Historical Dictionary of Italian Cinema. Scarecrow Press, 2008.

External links

1939 films
Italian comedy films
1939 comedy films
1930s Italian-language films
Films directed by Carlo Ludovico Bragaglia
Italian black-and-white films
1930s Italian films

redpajama_set_name: RedPajamaWikipedia


Büşra A. • Ekim 18, 2016Menude olmayan bi kokteyl yaptirdim harikaydi. Cok cesit var, herkes memnundu. Ortam da nezih.
Jean-Paul S. • Mart 21, 2017Lovely bar with great cocktails that are not expensive at all (11 euros). Open in the weekends, worth a visit!
María d. • Mayıs 30, 2017It opens until 2am. Alternative place in Amsterdam, they have good beers, shows and a dance floor. One of my favorites.
Yulia R. • Ocak 17, 2018Nice and cozy bar with creamy cocktails and snacks!
Rewan P. • Aralık 12, 2016Excellent views with outdoor seating available during summers. They have great music and cocktails. They have a lot of seating.
Titouan D. • Ocak 27, 2013sweet music, sweet cocktails, awesome people!
Lynn B. • Kasım 7, 2018Modern lunch spot at the Rokin, the touristic heart of Amsterdam. Good and tasty sandwiches and attentive staff!
Fanni L. • Şubat 23Amazing experience with this new place in Amsterdam. Great drinks and music. Hope to come back soon, highly recommended!
Marijn L. • Şubat 20, 2015Had an excellent five-course-dinner here. Super friendly staff, great food with loads of vegetarian options. Make sure to make you're reservation for after eight. As that's when it gets crowdier.
Deepesh B. • Ağustos 18, 2018Tried beet jerky. Very unique cocktails!!
Nikola R. • Nisan 21, 2015Cute place with an interesting twist to an anglo-american brunch/lunch menu - guess you can't go wrong with whatever you order.Great chai latte and machiatto, Friendly staff as well.
Maria A. • Haziran 5, 2013Beautiful Hotel at the Keizersgracht very central located. Cozy and nice design and a helpful and friendly Stuff! We will come back!
Jean-Paul S. • Mart 4, 2015Cosy cocktailbar with awesome food. From nachos to dinner, it's all a good idea at Snappers. Lovely pornstar martini, rest of the menu is perfect as well.
Sitki Cagdas I. • Ekim 24, 2014Binbir çeşit aromayı önce koklayarak tanımak, sonra da bu aromaları içeren kokteyllerden seçim yaparak tatlarını deneyimlemek... Mutlaka Amsterdam'a gelinirse uğranılması gereken bir mekan.


AFRICA and the MIDDLE EAST :: Where the Heck is Mom?
From Johannesburg, Clarens and the Drakensbergs, Golden Gate Highlands National Park and Royal Natal National Park, guest farm stays, Durban, the St Lucia area including Hluhluwe-iMfolozi and iSimangaliso Wetland Park.
Sixteen nights safari with Bushways, in a TENT.
Livingstone, Lusaka, 'Up Country' with the Peace Corps and Approriate Technology, and the Chimfunshi Wildlife Orphanage.
I see why everyone who comes here loooves Cape Town.
Including East Jerusalem, Masada, the Dead Sea.
Caesarea, Haifa, Tel Aviv-Jaffa, and Akko.
My two ten hour flights (LA-Amsterdam-Johannesburg) were, seen together, a singular miracle. I can�t imagine how the outcome could have been anything but a miracle. I did wear my high tight wool socks which I think might have made for happy legs and warm feet, not a miracle there. The miracle was my seatmates. On both flights my seatmates kept their entire body in their own seat and stayed on their own side of the arm rest. We took little elbow turns but not by hanging over the whole arm rest, no, no. They didn�t play loud music, or jiggle around, or talk excessively or loudly, they were perfect. Twenty hours in the air in coach, packed to the rafters with every seat taken, and at the end I wasn�t even agitated, I threatened no violence, I was ok. WOW, a MIRACLE!
Then I walked directly to the in-airport City Lodge Hotel where you pay a premium for the convenience but it was quite nice and well worth it. I went immediately into the bed and woke up 13 hours later. Not what I had intended but I was certainly refreshed!
I walked back into the totally modern airport to get cash (easy-peasy), rent a phone (that I haven�t tried yet), get a thing for my computer to connect to the internet (that isn�t working), get a gps (that isn�t charging properly and could quit at any moment), and rent the car. This whole process took a couple of hours plus the late start meant that I was going to be driving most of the way to Clarens in the dark. It�s the thing I always say I never want to do � drive in the dark. But as all my dear friends know when they tell me what they are never going to do, I also always say never say never. It was ok, not my favorite.
During the two hours of daylight that I did have the scenery was entirely Big Sky, that 360 degree view of the horizon. A problem when driving yourself is getting the shot. It seems you can get any shot you want, just stop and get it but you can�t stop on the big roads because of all the traffic and you can�t stop on the small roads because there isn�t any shoulder. I did grab a couple shots out the window, this being one.
Clarens �The Jewel of the Free State� is a sweet little town and I�ll tell about it tomorrow when I have some daylight pictures. I knew they had guest houses all up and down the main street and had a couple in mind so when I came upon my number one choice, the Rosewood Corner Guesthouse, they had a room and I took it. It�s perfect AND they are across the street from a perfect restaurant.
I must mention the stars since I'm always on about them. NOW we're talkin' STARS...the sky so dark the Milky Way so bright. I gasped!
The restaurant�s name is 278 on Main and it was perfect for me, warm and lively inside, great staff, delicious food. My first meal in South Africa turned out to be a total pleasure.
The vegetables were fresh and perfectly done. The green beans were lightly steamed, the beets were baked, the butternut squash was pan fried in butter for a nice crusty bite. The main dish is called bobotie (pronounced ba-boor-tea). a ground beef dish with condiments. I got it because it was their South African specialty. I got a glass of the local wine too (tasty!) so the staff were all anxious to hear my report.
I�m anxious to get out and look around so I�ll probably leave the hassle with the internet card and the gps for later. Guess I�m going to buy a map!
Here are some views of the Rosewood Corner B&B in Clarnes.
At breakfast there was cold cereals out as well as toast, preserves, orange marmalade (yum) freshly cut fruit and a passion fruit yogurt that was so good I had to eat it twice. Then our host asked if we�d like a hot breakfast. Perfectly satisfied as I was I was not going to turn down scrambled eggs with herbs and cheese, broiled tomato, and stripy bacon (English style but cooked the way I like it). Oh yeah.
Here are a few views around Clarens this bright and Freezing Cold morning. It's the central plaza and yes, it�s SNOW.
You can see from the signs that the town focuses on galleries, B&Bs, and restaurants and cafes.
I took one of the towels from my room to wrap around my neck when I went out at 6am for these pictures.
My room was only barely warm but they had a mountain of quilts and an electric blanket under the bottom sheet, so aside from wearing all my clothes all the time and not wanting to take a shower and using a towel for a scarf, I was perfectly fine.
It's a pretty little town and very conveniently located between Jo'burg and the Drakensbergs to keep any one day's drive under four hours. My goal.
It didn�t look like that when I was there but it was lovely none the less and I could see the hints of the colors to come.
Coming next into Royal Natal National Park to admire the postcard destination, the Amphitheatre. Royal Natal (btw every time you see Natal pronounce it naTAL) is a small park that is part of the UNESCO World Heritage uKhahlamba-Drakensberg Park. The Drakensbergs overall are supposed to be amazing to visit but I�m probably not going to devote another day to the area but rather move on to Durban.
What some of the National Park lodging looks like. It's actually quite expensive to stay inside any of the parks and the hot tickets like Kruger in season you have to make reservations well in advance.
Helmeted Guineafowl. They are everywhere. I heard that they are particularly tasty stewed in a pot of red wine.
Tonight�s accommodation: Dalmore Guest Farm outside the town of Bergville and 6 kilometers down a dirt road. What an excellent choice I made randomly off the internet!
They have a lot of rondavels on this property for all kinds of uses which reminds me that I don�t have any pictures of the townships where you find rondavels and structures put together from every other type of building material. Every hour or two while driving along in the countryside out of nowhere, just there, will be a huge collection of very poor dwellings, as far as you can see. I was thinking how to manage a visit but a plan has not yet come to mind.
Around the property. There are farmers of many description and also livestock. Here they keep sheep and plenty of them.
No lions or leopards yet, but we've got lambs!
Kaitlin - which of these two pictures do you like better? This one?
Another of the rondevals in the background with the traditional straw roofing. They are doing some building projects here in the local style and when I get a chance I'll add some pictures.
Dinner at the big house.
The kids ate first. This is five of the seven children under the age of 9.
All the other guests were local people. I stayed up later than usual and had to at least try the local beverages (don't forget to ask Lill about...is it glog?). It was a most lively and entertaining evening.
And much to my delight she said 'go to Durban and then stay the night at our place.' She didn't have to ask me twice!
Durban is most well known I think for three things. 1) is the largest population of people of Indian decent in South Africa, the most in any city outside India according to Heather's husband Martin.
It was a train ride from Durban to Pietermaritzburg that was one of the seminal moments in Gandhi's political life, when he was not allowed to travel on the first class ticket bought for him by his employer.
2) Surfing. The water is warm all year and the waves are consistently large and well-formed.
...and looking in the other direction.
Then I met up with Heather and her seemingly sane/urbane/yet tearing around on a motorcycle-maniac husband, Martin. We ate dinner at an Indian restaurant of which there are so very many because of point 1) above.
I got to have something I'd never had before and is one of the staples of Indian restaurants in South Africa. I ate a bunny. A bunny is either 1/4 or 1/2 or 1 whole loaf of dense white bread hollowed out with a curry poured in and a bit of the inside bread positioned on top I think, just guessing, to represent a little cottontail. It was, in fact, delicious.
Their home is a huge rambling English Tudor Revival(?) on the top of one of the hills overlooking the sea. The house was built about one hundred years ago as a home for Standard Oil executives.
The big eat-in kitchen and a selection of Heather's heart collection.
Heather's office downstairs. She is both a painter and a photographer and get this, she makes money from her work. Weddings are the bread and butter of the business but she does a lot of other projects too.
I like how she adds painting to the wedding albums.
I heard so many interesting stories - about the kids, the business and household staff, Martin's work, and generally how it is to live in South Africa. Lucky me or what.
The view from their back windows and garden.
The 8th has been a driving-getting settled-no-photo day but tomorrow, the 9th, finally - wild animals! at the Hluhluwe-iMfolozi Game Reserve. I'm getting picked up at FIVE AM. Yikes.
Meet the team for the safari tour through the Hluhluwe-iMfolozi (pronounced Shlushluwee) National Park, the oldest National Park in Africa. The couple on the left are tourists from Durban and the four women on the right are volunteering for a few weeks at a health clinic in Saint Lucia.
You can see the vehicle in the background. Most of the time it was raining hard and the wind whipped through the plastic coverings and it was cold...yikes. But wow, everyone (even me mostly) kept up good cheer. Thankfully the rain stopped just in time for lunch.
After our 5AM pickup from various guest houses we got this lovely sunrise more than an hour later.
Look! In the bush over there, White Rhinos!
From Ms Wiki: "The park is the birthplace of rhino-reservation, breeding the species back from extinction (less than 20 (white) rhinos world wide in 1900 to more than 10,000 today). As the home of Operation Rhino in the 1950s and 60s, the Park became world renowned for its white rhino conservation.
"The Rhino Capture Unit of the park can take credit for helping save the endangered White Rhino from the brink of extinction. Today the reserve has over 1600 white rhino in the reserve and has relocated hundreds of these magnificent animals to game reserves around the world."
And mama and daughter are gone.
Warthogs. They do have wart-like protuberances and according to the guide they taste like delicious hogs.
Two wiki-facts: a group of warthogs is called a sounder; the warthog is the only pig species that has adapted to grazing.
Africa's traditional Big Five, all found here: Elephant, Rhinoceros, Cape Buffalo, Lion, Leopard.
This is a Cape Buffalo. We never found an elephant or a leopard.
I'm not seeing these guys in the naming chart...I'll have to ask someone.
I did see both a male and a female Nyala but their pictures are fuzzy, and some fuzzy Reedbucks too. No Impalas and no Elands though. According to the naming chart these are all variates of antelope.
Gnu. Of course everyone had to call out 'who gnu?'. They are also called Wildebeest.
It's winter in South Africa now and the grasses have died back and the deciduous trees have lost their leaves making the animals easier to spot than in summer when the landscape is lush and beautiful.
I'm leaving the darkness so you can get a feel for what it looked like pre-photoshop.
I'd moved from the back of the truck to the front seat to warm up. Wet and warm was far more comfortable than wet and cold although I did lose the height of the back of the truck.
Giraffes in the distance. So Africa.
Check out the little birds with the red heads, four of them, grooming the giraffe.
Cheetah! This was exciting. Cheetahs are about half the size of leopards and as a matter of fact, cheetahs weigh less than I do.
Stop now, baboons crossing. Check out the mama with her baby on her back.
The rain stopped in time for our lunch which was a great delight - the first picture in this set is from our braai. Braaivleis is Afrikaans for grilled meat and a braai picnic, like a bbq, is hugely popular.
According to the guide that littlest one is less than one day old. It was such a surprising sight the guide got out his camera.
Bye Hluhluwe-iMfolozi, it's been great!
I got back to my wonderful accommodation, fell into bed, and slept for several hours before tackling these pictures. Now it's time for bed again!
Elephant Coast Guesthouse (their banner btw-I didn't pick that font!), the place where I'm staying for three nights in St Lucia, and that's my room featured. There's also a lounge area in the room with comfy chairs and a reading light. I'm very happy here.
Following are more animals. This is going to be the last hit of animals until I get to Botswana, and I deleted a few pictures from yesterday...I know, still too many animals.
Hippos and what a great sound they make.
I'm doing a self-drive-tour through the highways and byways of one section of the iSimangaliso Wetland Park, a UNESCO World Heritage site.
They've got everything at iSimangaliso but are especially rich in the variety and quantity of birds. I cannot ever Ever get a bird to be in focus so no photos, but it is true, they have got some serious bird action going on here.
A Vervet monkey. There are also Samango monkeys in the area . . and which is which?
The St Lucia estuary, and where I drove, is a bit of land with the Indian Ocean on one side and the largest salt water lake, St Lucia, on the other.
From Ms Wiki: "The reason for the huge diversity in fauna and flora is the great variety of different ecosystems on the park, ranging from coral reefs and sandy beaches to subtropical dune forests, savannas and wetlands."
Red duiker. Hi little guy.
I did walk out there, carefully... This is on the lake side, the wetlands.
Kudu - quite the handsome fellow.
...and another waterbuck. Maybe the ones above are the females and this guy is a male. I'd expect those horns are quite valuable.
I think he might be a black rhino and not the white one from yesterday? You can be 100% sure the car will wait and the rhino will decide the next move. I came upon the scene and was far enough away to be able to back up slowly and then get the heck out of there.
Should that rhino take it into his bitty brain to charge the car - goodbye car.
The sand dune area is huge, this is just a slice, and the color is true to life.
Wildebeest or more Cape Buffalo?
A near sunset scene of zebras, warthogs (or are they bushpigs?), and some kind of antelope grazing together for fresh sprouts in a recently burned field.
There are grazers who go for the grasses and browsers who go for leaves and fruits. This is vocabulary I have learned and forgotten dozens of times.
For the evening I picked up a pre-made salad at the market, did pictures, and listened to NPR on the computer. Ahh, nice.
These two days were mostly driving so I'm going to talk about driving in South Africa now.
SA is a drive-on-the-left country which means the driver sits on the right side of the car which means you operate the stick shift with your left hand. Left handed shifting! But stick shift cars are half the price for twice the power and I don't mind. So far so good. .I just have to get to the airport in the morning without incident and all will be well.
The main roads are basically ok - the toll roads especially. But I spent an enormous amount of time sitting in line-ups, waiting turns during road work when only one lane was available. SO so much road work.
And many of the roads not being worked on are badly torn up with potholes. Then there's all the trucks, which on the two lane roads means constant passing into on-coming traffic. Between the road work, the potholes, and the trucks every journey took much longer than I at first thought it would.
Still, except for this afternoon in Jo'burg which was very tough, the driving has been just fine and really the only way to get around.
Always a welcome sight. Toilets, snacks, the omnipresent Wimpy.
hWhat you're seeing here is a small residential compound at the edge of the farm where I spent the night. There are similar groupings all along the road, and you can take this place and multiply it by hundreds to get an idea of some of the more extended (entirely black) communities.
It has been less than 20 years since the Apartheid system was law, not so long ago. I didn't know it at the time, when I was working out this trip and choosing accommodation, and in retrospect I can see how it happened, but I didn't expect that I would find myself basically surrounded by only white people as owners, guides, etc. (10% or so of the population) and only black people in service roles. Not to say that this is not entirely true of everywhere of course, just where I was.
My plan to keep each day's drive to four hours was a good one since what googlemaps said would take four hours actually took more like six.
Travelling from St Lucia back to Jo'burg I chose another farm stay to break up the drive. This is the big house.
The name of the B&B business, not the farm, is 'Dusk To Dawn' 20 kilometers or so outside Piet Retief, and my accommodation was bigger than my house.
One of the dogs went with me for a late afternoon stroll.
They have many enterprises here including a lot of livestock, mostly pigs and cows, and a timber business farming eucalyptus and pine.
Morning from my bedroom window. After a delicious farm fresh breakfast I left for what was to be a four and a half hour drive that ended up being six and a half hours to get to where I was going in Jo'burg.
But eventually I made it to the nighborhood where I was intending to stay at one of the several guesthouses, and after looking at a few found one, The Sleepy Gecko, that was just the ticket.
...on 7th Ave in Melville.
I drove many many miles around Jo'burg in all my wrong turning and highway errors and truth be told it is mostly not a place to be out in after dark. Even Lonely Planet which is generally a go-for-it publication urges caution and has very few accommodation suggestions in the whole city but does recommend this little enclave as a good place to visit.
It is a very cool little four block community.
I have to get up and out early tomorrow to get to the airport to catch my flight to Maun.


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While some people have the general belief that a dog is a man's best friend, others feel the urge to buy monkeys.
Although the interesting creatures can be purchased as pets in many countries, the laws in the United States require an owner to have a proper permit to own the animal. Chris Brown must have missed that part of his monkey manual though.
Chris is in trouble with the law yet again. This time though, the charges stem from the talented singer's pet monkey. As reported by TMZ, the Los Angeles City Attorney's Office is charging Brown with two counts of owning a restricted species without a permit.
The violations carry a maximum sentence of 6 months in jail. Brown brought home the baby capuchin monkey named Fiji and allowed his daughter to play with the pet on his social media. If you recall, that wasn't well accepted.
Chris was forced to give up the pet after a horde of people online reported him to the authorities. At the time, which was at the top of 2018, we reported that he would possibly get hit with criminal charges.
Those charges have finally been filed. Breezy is due in court on February 6, and hopefully, he's only hit with a few fines.


text:
celebrities, danai gurira, Editorials, Fashion, PorterEdit
Danai Gurira for PorterEdit April 2019. Images by Claire Rothstein.
danai gurira, Editorials, Fashion, SHAPE
Danai Gurira Covers SHAPE Magazine May 2019. Images by James Macari.
Activewear, black panther, danai gurira, Reebok, The Walking Dead
Danai Gurira Stars in Reebok Campaign.
celebrities, danai gurira, Editorials, Fashion, Women's Health
Danai Gurira Covers Women's Health July/August 2018. Images by Ben Watts.
Bustle, danai gurira, Editorials, Fashion
Editorials. Danai Gurira for Bustle. Images by Meredith Jenks.
danai gurira, Film, Film-News
Danai Gurira Set to Star in 'Avengers: Infinity War.'
celebrities, danai gurira, Fashion, The Walking Dead, Thom Browne
Danai Gurira Wears Thom Browne to the 'Talking Dead.'
Atlanta Magazine, celebrities, danai gurira, Editorials, Fashion
Editorials. Danai Gurira. Atlanta Magazine. Images by Alex Martinez.
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Danai Gurira Features in Harper's Bazaar. Talks Identity.
2016 Obie Awards, danai gurira, Fashion, Lupita Nyong'o
On the Red Carpet. Lupita Nyong'o and Danai Gurira at the 2016 Obie Awards.
celebrities, danai gurira, Editorials, Fashion
Snapshots. Danai Gurira for The Edit May 2016. Images by Bjorn Iooss.
Conan, danai gurira, Michonne, Tattoos, The Walking Dead
Michonne Tattoos Are Very Much a Thing.
tattoo image via Tattoo.com

redpajama_set_name: RedPajamaCommonCrawl


text:
import { compose, createStore, applyMiddleware } from 'redux';
import { reduxReactRouter } from 'redux-router';
import createHistory from 'history/lib/createHashHistory';
import reducer from '../reducers';
import layerMiddleware from '../middleware/layerMiddleware';

export default function configureStore(layerClient, initialState) {
  const finalCreateStore = compose(
    applyMiddleware(layerMiddleware(layerClient)),
    reduxReactRouter({ createHistory })
  )(createStore);

  return finalCreateStore(reducer, initialState);;
}

redpajama_set_name: RedPajamaGithub


Our classic polo in a soft navy knit makes a perfect Spring or Summer "go to" for your little boy. Add a monogram to personalize.
If you do not purchase the Monogram Add On,your item will ship without being monogrammed.


A bye week 4 weeks into the season is a bit early. However, the early week off appears to have been a blessing in disguise for the Carolina Panthers. As of the end of practice last weekend, the team was without Curtis Samuel (medical illness), safety Da'Norris Searcy and tackle Daryl Williams (IR), and Greg Olsen (foot).
Over the break, the Panthers signed safety Eric Reid to a one-year deal and traded for tackle Marshall Newhouse. When the team took the practice field Monday morning, Curtis Samuel and Trai Turner were both back in action while Olsen worked off to the side with trainers – still a good sign.
Reid was also asked about his emotions leading up to getting back on the field. He stated that it happened quicker than he thought and also disclosed that he signed with the Panthers over the 49ers because "it was a better deal." Reid also says that the Panthers did not ask him about his plans or methods of protest before signing him. Prior to the start of the season, the safety had revealed that he is still considering how he will protest this season.
When asked if protesting was worth the risk of losing his football career, Reid cited mass incarceration and systematic oppression as just a few reasons why he protests. He also cited the recent killing of Botham Jean who was murdered in his own home.
Flip the page for snippets from Monday's press conference.


The 10th Annual ASDA'A Burson-Marsteller Arab Youth Survey 2018 was conducted by international polling firm PSB Research to explore attitudes among Arab youth in 16 countries in the Middle East and North Africa. PSB conducted 3,500 face-to-face interviews from January 21 to February 20, 2018 with Arab men and women in the age group of 18 to 24. The interviews were completed in Arabic and English.
The aim of this annual survey is to present evidence-based insights into the attitudes of Arab youth, providing public and private sector organisations with data and analysis to inform decision-making and policy formation.