text:
\section{\protect\normalsize INTRODUCTION}

Quantum networks are the platform for the implementation of quantum communication and quantum information processing \cite{1}. They comprise of local network nodes, which are capable of efficient storing, processing and releasing photonic quantum information in a reversible fashion, and of quantum channels, which link the memory nodes by transmitting photonic states between them with high fidelity of the transfer. The original proposal for the quantum state transfer (QST) is based on the "single atom-optical cavity" system \cite{2}, where the reversible mapping of quantum states between light and matter is achieved due to the strong coupling of the interaction of single atoms and photons, while quantum channels, for example optical fibers, coherently exchange single photons between different nodes. The remarkable capability of this scheme to connect distant quantum objects, stimulated many efforts aimed at solving the main challenges in quantum information transfer between remote qubits. Specifically, new schemes have been developed for robust creation and storage of quantum entanglement over long distances \cite{A,B,C,D}, heralded storage of polarization states of single photons in single atoms \cite{E,kurz,F}, quantum error correction \cite{G}, implementation of quantum gates between distant atoms \cite{H}, single-photon generation \cite{I, J, K}, faithful and controllable matter-light quantum interfaces \cite{L, M} including those based on optomechanical transducers \cite{N}. Utilizing the global resources of this scheme, a new quantum protocol have been offered for a network connecting the geographically remote optical atomic clocks \cite{O}.  Inspired by the proposal of Ref.\cite{2}, where the atom-cavity system produces a time-symmetric photon wave packet to prevent the photon reflection from the second cavity mirror, a different approach was suggested in \cite{P} based on an adiabatic passage through a dark state of both cavities that reduces the cavity photon losses. The first implementation of the scheme in Ref.\cite{2} with direct, albeit probabilistic, connection of the states of two distant atoms was presented in the recent paper \cite{3}, which combines in one experiment the basic operations that have been previously realized separately with cavity QED including the interconversion of photonic and atomic quantum states \cite{4,5} and generation and storage of cavity photons in a single-atom quantum memory \cite{6}. However, the  efficiency of the QST currently available in this scheme is rather low to implement scalable quantum networks, as a desired result is obtained only after many unsuccessful attempts requiring much more time as compared to the realistic quantum memory lifetimes. These difficulties are typical also for the entanglement swapping in probabilistic protocols for quantum repeaters \cite{7}. For the full employment of quantum networks, new schemes with highly efficient emission and storage of cavity photons, as well as low-loss photonic links between the cavities are required. Recently, the deterministic transfer of microwave photons and entanglement generation between distant superconducting qubits have been demonstrated in a number of works \cite{8,9,10}, but the reliable exchange of optical photons between spatially separated nodes still remains a challenging task.

In this paper, we propose a quantum network protocol based on the deterministic generation and absorption of cavity photons in network nodes, which consist of single $F$-Zeeman-structured multilevel atoms, with $-F\le m_F\le +F$, confined in identical single-mode high-finesse optical cavities. In the sending node, an arbitrary quantum state is encoded in the superposition state of the ground Zeeman sublevels of the single atom, which strongly interacts with linearly polarized cavity mode and a circularly $\sigma^+$ polarized control $\Omega_1(t)$ laser field in a Raman configuration. The control field transfers the atomic population into the extreme Zeeman state $m_F=+1$ via Raman transition and, thus, completely converts the atomic superposition state into PNSS of linearly polarized cavity photons.  Note that the schemes enabling atomic ground-state Zeeman coherence to be mapped onto the cavity-mode field using the adiabatic passage have been studied in \cite{first,second}. In our case of Raman configuration the temporal profiles of the photons are determined by the shape of laser pulse. This process is deterministic due to the very high signal-to-noise ratio that is available in real conditions. We first consider the simple case of the atomic $F=1\rightarrow F'=2$ transition, when the atom is initially prepared in an arbitrary superposition of ground Zeeman states $m_F=-1$ and $m_F=0$ (Fig.\ref{fig:fig1}, left), where the photonic qubit as a superposition of one- and two-photon states is generated, which identically reproduces the form of atomic superposition state. An external magnetic field applied perpendicular to the cavity axis removes the Zeeman degeneracy in such a way as to fine-tune the linearly polarized cavity mode to the exact resonance with two-photon Raman-transitions, as well as to reduce the decoherence of the atomic superposition by ambient magnetic fields. The photons leave the cavity through one mirror, which is partially transparent, as a freely propagating wave packets, which are efficiently coupled to a low-loss single-mode optical fiber. The latter transmits the photons to the receiving system (Fig.\ref{fig:fig1}, right), where a single atom is prepared initially in the state $m_F=+1$. The atom interacts with a circularly $\sigma^+$ polarized $\Omega_2(t)$ laser field, which induces coherent absorption of incoming photons with unit probability, eventually settling down the receiving atom into the same superposition state as the original one in the sending system. The shape of the $\Omega_2(t)$ laser pulse is derived from the requirement to entirely exclude the photon leakage from the second cavity indicating that the quantum output field is zero at all times. We show that the absorption amplitudes are not sensitive to the photons' temporal shape due to integral dependence on the latter (see Sec.IIIB) that significantly alleviates the strict condition of high transfer efficiency requiring the photons of time-symmetric shapes \cite{2,11}.

Further we extend the developed technique to the case of the QST by the photonic qutrit, which is a superposition of the vacuum, one- and two-photon states and possesses greater information capacity, whereas the quantum connectivity between the nodes using this state is not less protected from the decoherence induced by the environmental effects than the photonic polarization qubit \cite{3}. With reduced photon losses in quantum channels, this deterministic protocol provides very fast and robust QST over large distances that notably mitigates the limitations on the quantum memory lifetime. Under these conditions the imperfection associated with the delivery of more than one photon does not reduce the final state fidelity.
\begin{figure*}[t] \rotatebox{0}{\includegraphics*
[scale =0.7]{Fig1.eps}} \caption{(Color online) (a) Quantum state transfer between two single-atom network nodes. The insets show the atomic level structure and transitions in the laser fields $\Omega_{1,2}$ and in an external magnetic field B. The sequent photons (thin red lines) are generated in the left and absorbed in the right cavities. The initial populations of atomic states are shown by filled circles \label{fig:fig1}}
\end{figure*}

This paper is organized as follows: In the next section, we present the interaction setup and derive the basic equations for the time evolution of the atomic state amplitudes and the cavity field, which describe the generation of PNSS of linearly polarized cavity photons in the sending system. We analyze the dynamics of atomic population and photon number distribution via numerical calculations, as well as we obtain the temporal profiles of emitted photons. Here we also estimate the error due to the spontaneous losses and discuss the main approximations ensuring the deterministic generation of PNSS. The analytic solutions for the coherent absorption of PNSS in the receiving system are found in Sec.III, where the final superposition state of the second atom is demonstrated. Here we also present the implementation of the QST via photonic qutrit. We discuss also the advantages and imperfections of our protocol in the Sec.IV and summarize the results in Sec.V.

\section{\protect\normalsize PNSS GENERATION IN THE SENDING NODE}

\subsection{Model}
The present mechanism for producing PNSS is based on our earlier proposed method of deterministic generation of a stream of multiphoton pulses in a single-atom-single-mode cavity QED system \cite{12,13}. A multi-level atom or ion is trapped in a one-mode high-finesse optical cavity and interacts with a $\sigma^+$-polarized laser field $\Omega_1$ (Fig.\ref{fig:fig1}a) on the multi-level chain, for instance, on the transition $5S_{1/2}(F = 1) \rightarrow 5P_{3/2}(F' = 2)$ of the $^{87}$Rb atom, where the state $5P_{3/2}(F' = 2)$ is well isolated from other hyperfine levels. The laser field couples the ground state $F=1$ with magnetic quantum number $m_F = -F,\cdots,F-1$ and the excited state $|F' =2, m_{F'} = m_F+1\rangle_1$ and creates a linearly polarized cavity-mode Stokes-photon (shown in Fig.\ref{fig:fig1} by red thin lines) on the transitions $|F' =2, m_{F'} = m_F+1\rangle_1 \rightarrow |F =1, m_F+1\rangle_1$, thus transferring the atom into the next Zeeman sublevel with $m_F+1$.  The one-photon blue detuning of the laser field, which is the same for both atoms $\Delta_1$=$\Delta_2$=$\Delta$, is taken very small compared to the upper level hyperfine splitting, but at the same time it is much larger than the cavity decay rate $k$, the natural spontaneous decay rate $\gamma_{\text{sp}}$ of the atom and the Rabi and Larmor frequencies: $|\Delta| \gg k, \gamma_{\text{sp}}, \Omega_{1}, \Delta_B^{(F, F')}$, where $\Delta_B ^{(F,F')}=g_L ^{(F,F')}\mu_B B/\hbar$ is the Zeeman splitting of the ground and excited states in the magnetic field $B$, with $g_L^{(F, F')}$ the Land\'e factor and $\mu_B$ the Bohr magneton. This condition allows one to suppress the off-resonant excitation to nearby hyperfine state $F'=1$ and, hence, to neglect the spontaneous losses from upper levels and dephasing effects induced by other excited states. In this far off-resonant case and for slowly varying laser fields: $d\Omega_1 / dt \ll \Delta\Omega_1$, one can adiabatically eliminate the upper atomic states that leads to the effective Raman atom-photon coupling
\begin{equation}
G_1=g\Omega_1/\Delta,\label{eq:1}
\end{equation}
which can be made much weaker than the cavity field decay: $G_1\ll k$. This ensures that the generated photons leave the cavity without being reabsorbed by the atom, resulting in the deterministic emission of photons. For simplicity, we assume here that the dipole matrix element $\mu _{F,F'}$ of the $F\leftrightarrow F'$ transition does not depend on the magnetic quantum numbers. This actual dependence can be easily taken into account in the numerical simulations \cite{13}.

The external magnetic field taken as the quantization axis is applied orthogonal to the cavity axis and parallel to the laser pulse propagation. As we mentioned in the introduction, it is chosen strong enough to preclude the generation of $\sigma^+$ and $\sigma^-$ polarized cavity photons due to the off-resonance interaction with the atom, which is the case if $\Delta_B^{(F)}\gg k$. This clearly increases the probability of photon production with linear polarization unlike the model considered in Ref.\cite{3}, where the generation of cavity photons with undesired polarization cannot be suppressed.

We describe the dynamics of the system in the Heisenberg picture. The pumping laser field is given by
\begin{equation}
E_1(t)={\mathcal E}_1f_1^{1/2}(t)\exp (-i\omega t)+h.c.,\label{eq:2}
\end{equation}
where $f_1(t)$ features its temporal profile of duration $T_1$ and ${\mathcal E}_1$ is the peak amplitude of the field with one-photon detuning $\Delta=\omega - \omega_{FF'}$ and the peak Rabi frequency $\Omega_1=\mu_{F,F'}{\mathcal E}_1/\hbar$.

After eliminating the upper states by virtue of large one-photon detuning, the effective interaction Hamiltonian in the RWA takes the form
\begin{align}
H&=\hbar \Biggl[\sum_{m_F=-F}^{F}\biggl ( \frac{g^2}{\Delta}a_1^{\dag}a_1+f_1(t)\frac{\Omega_1^2}{\Delta}\biggr )\sigma_{m_F,m_F} \nonumber \\
&+ G_1 f_1^{1/2}(t) \sum_{m_F=-F}^{F-1}\biggl (a_1^{\dag}(t) \sigma_{m_F+1,m_F}(t)+h.c.\biggr )\Biggr],\label{eq:3}
\end{align}
where $\sigma_{i,j}(t) = |i \rangle_{11}\langle j |$ and $a_1(t)$, $a_1^\dag(t)$ are correspondingly the atomic and photonic mode operators in the first cavity. The first and second terms in Eq.\eqref{eq:3} describe the Stark shifts of atomic ground states induced by the cavity field and laser pulse $\Omega_1$, respectively. Under the adopted approximation of equal dipole moments, the Stark shifts induced by the laser field have no influence on the photon  generation, since their difference between two neighboring atomic ground states is zero for all transitions $m_F  \rightarrow m_F + 1$. On the other hand, the Stark shift $g^2/\Delta$ can be included into the cavity mode frequency: $\omega_c \rightarrow \omega_c-g^2/\Delta$. Below we use these simplifications to get the analytic solution revealing the main features of the system considered. In real atoms, where the dependence of $g$ and $\Omega_1$ on Clebsch-Gordan coefficients leads to non-vanishing Stark-shift difference, the latter can be made negligibly small as compared to the cavity decay rate $k$ by appropriately choosing the system parameters \cite{13}.

\subsection{Dynamics of atomic populations}

The production of PNSS from the first cavity starts by preparing the single atom in a superposition of the states $|F=1,m_F=-1\rangle_1$ and $|F=1,m_F=0\rangle_1$, denoted below as $|-1\rangle_1$ and $|0\rangle_1$, respectively, with normalized population amplitudes $c_{-1,0}: |c_{-1}|^2+|c_0|^2=1$, while the cavity mode is in the vacuum state. Then, the initial state of the sending system can be represented as
\begin{equation}
|\Psi_{\text{1,in}}\rangle=\biggl (c_{-1} |-1\rangle_1 + c_0 |0\rangle_1\biggr ) |0\rangle_{1c},\label{eq:4}
\end{equation}
where $|0\rangle_c$ refers to the state of cavity with zero photon number.

The applied $\Omega_1$ laser field transfers the atom to the final state $|F=1,m_F=+1\rangle_1=|1\rangle_1$ in two steps (if $c_{-1}\neq 0$), each time generating via Raman process a linearly polarized Stokes photon (Fig.\ref{fig:fig1},left).

The equations for the Zeeman sublevel populations $\langle\sigma_{m_F}(t)\rangle \equiv \langle\sigma_{m_F,m_F}(t)\rangle$ and ground-state coherence $\langle \sigma_{m_F,m_F+i} (t) \rangle=\langle \sigma^*_{m_F+i,m_F} (t) \rangle, i\neq 0,$ were derived in our previous papers \cite{12,13} from the master equation for the whole density matrix of the system.  The Hamiltonian \eqref{eq:3} and the input-output relation $a_{1,\text{out}}(t)-a_{1,\text{in}}(t)=\sqrt{k}a_1(t)$ \cite{14} for the photonic operators were used in the adiabatic limit $kT_1\gg 1$, where the cavity mode operator $a_1(t)$ is expressed through the atomic operators as
\begin{equation}
a_1(t)=-\frac{2i G_1}{k} f_1^{1/2}(t)\sum_{m_F=-F}^{F-1}\sigma_{m_F+1,m_F}(t) - \frac{2}{\sqrt{k}}a_{1,\text{in}}(t).\label{eq:5}
\end{equation}
In the sending node, the input field $a_{1,\text{in}}(t)$ is in the vacuum state $\langle a^{\dag}_{1,\text{in}}(t) a_{1,\text{in}}(t)\rangle = 0$ and will be ignored in further calculations.

In general, the atomic equations contain all relaxation processes including the optical pumping from $|F,m_F\rangle_1$ into states $|F,m_{F}+i\rangle_1, i = 1,2$, and the losses of atomic populations due to the decay from the upper atomic states into the states outside of the system. However, the deterministic production of cavity photons requires that the total spontaneous loss is negligible, which is achieved, if $\alpha_1f_1(t)\gg\Gamma_1(t)$, where $\alpha_1=4G_1^2/k$ is the cavity photon generation rate and $\Gamma_1(t)=\frac{\Omega_1^2}{\Delta^2}f_1(t)\gamma_{\text{sp}}$ is the total spontaneous decay rate induced by the $\Omega_1$ pump pulse. This defines the signal-to-noise ratio
\begin{equation}
R_{\text{sn}} = \frac{\alpha_1 f_1(t)}{\Gamma_{1}(t)} = \frac{4g^2}{ k\gamma_{\text{sp}}} \gg 1.\label{eq:6}
\end{equation}
This condition is clearly fulfilled in high-finesse optical cavity with $g > k, \gamma_{\text{sp}}$.

With this approximation the atomic equations are greatly simplified and for $F=1$ take the form
\begin{widetext}
\begin{subequations}
\begin{eqnarray}
& & \frac{d\langle \sigma_{m_F} (t) \rangle}{ dt}=\alpha_1f_1(t)[\langle \sigma_{m_F-1}(t) \rangle \theta(m_F)- \langle \sigma_{m_F}(t) \rangle \theta(-m_F)],\label{eq:7a}\\
& & \frac{d\langle \sigma_{m_F,m'_F} (t) \rangle }{ dt}= - \frac{1}{2}\alpha_1f_1(t)\biggl (\langle \sigma_{m_F,m'_F}(t)\rangle [\theta(-m_F)+\theta(-m'_F)] -2 \langle \sigma_{m_F-1,m'_F-1}(t)\rangle \theta(m_F)\theta(m'_F)\biggr ),\label{eq:7b}
\end{eqnarray}\label{eq:7}
\end{subequations}
\end{widetext}
where $\theta(x)$ is the Heavyside step function with $|m_F,m'_F|\leq F$ and $m'_F\neq m_F$.
One can easily check from Eq.\eqref{eq:7a} that the total population of atomic ground state is conserved:
\begin{equation}
\sum_{m_F=-F}^F\langle \sigma_{m_F} (t)\rangle  = 1.\label{eq:8}
\end{equation}

Equations \eqref{eq:7} are solved subjected to the initial conditions $\langle \sigma_{i}(-\infty)\rangle =|c_i|^2, i=-1,0$ and $\langle \sigma_{-1, 0}(-\infty)\rangle =c^*_{-1}c_0$, $\langle \sigma_{0,1}(-\infty)\rangle =\langle \sigma_{-1,1}(-\infty)\rangle=0$, which gives
\begin{subequations}
\begin{eqnarray}
& & \langle \sigma_{-1}(t)\rangle=|c_{-1}|^2 e^{-\vartheta(t)},\label{eq:9a}\\
& & \langle \sigma_0(t)\rangle=[|c_0|^2+|c_{-1}|^2 \vartheta(t)]e^{-\vartheta(t)},\label{eq:9b}\\
& & \langle \sigma_1(t)\rangle=1-(1+|c_{-1}|^2 \vartheta(t))e^{-\vartheta(t)},\label{eq:9c}\\
& & \langle \sigma_{-1,0}(t)\rangle=c^*_{-1}c_0 e^{-\vartheta(t)},\label{eq:9d}\\
& & \langle \sigma_{0,1}(t)\rangle=2c^*_{-1}c_0 (e^{-\vartheta(t)/2}-e^{-\vartheta(t)}),\label{eq:9e}\\
& & \langle \sigma_{-1,1}(t)\rangle\equiv 0,\label{eq:9f}
\end{eqnarray}\label{eq:9}
\end{subequations}
where the new variable
\begin{equation}
\vartheta(t) = \alpha_1\int \limits_{-\infty}^tf_1(t')dt'\label{eq:10}
\end{equation}
is proportional to the pump energy confined in the $(-\infty,t]$ area of the pulse.

For a Gaussian laser pulse of profile $f_1(t)=e^{-(t/T_1)^2}$ with duration $T_1=0.3~\mu$s, the atomic level populations are shown in Fig.\ref{fig:fig2}, where we have used the realistic parameters $(g, k, \gamma_{\text{sp}}, \Omega_1, \Delta^{F'}_B, \Delta) = 2\pi\times(12, 3, 5.87, 10, 15, 100)$~MHz \cite{15,16,17}, for which the signal-to-noise ratio in Eq.\eqref{eq:6} is $R_{\text{sn}} \sim 30$, thus justifying the approximation on neglecting relaxation processes. A magnetic field of $15$~G well resolves the Raman resonances, thus precluding the generation of circularly polarized cavity photons. There is a significant increase in the population of the state $|F=1, m_F=0\rangle_1 $ in the vicinity of $kt\sim-6$, which results from the population motion from the state $|F=1, m_F=-1\rangle_1$, while emitting the first photon. Yet, the both states are emptied almost simultaneously, which occurs already at the leading edge of the laser pulse. As shown in the next Section, this ensures simultaneous absorption of two photons, as a result the receiving atom settles in the desired superposition state.

\begin{figure}[h] \rotatebox{0}{\includegraphics*
[scale =0.7]{Fig2.eps}} \caption{(Color online) Populations of the ground Zeeman states $|m_F=-1\rangle_1$ (red),$|m_F=0\rangle_1$ (blue) and $|m_F=+1\rangle_1$ (black). The Gaussian laser pulse of FWHM duration 0.5~$\mu$s is shown by the dotted line.
The atom is initially prepared in the states $|F=1,m_F=-1\rangle_1$ and $|F=1,m_F=0\rangle_1$ with populations $|c_{-1}|^2=0.7$ and $|c_0|^2=0.3$, respectively. See the text for other parameters.
\label{fig:fig2}}
\end{figure}

After emission of photons, the sending atom passes to the final state $|F=1, m_F=+1\rangle_1$ (black line in Fig.\ref{fig:fig2}), where it continues to interact with the laser field on the transition $5S_{1/2}(F=1,m_F=+1) \rightarrow 5P_{3/2}(F'=2,m_{F'}=+2)$, neither emitting a cavity photon nor decaying into the outside state $5S_{1/2}(F=2)$ owing to the small value of $\Gamma_1$. Therefore, if the laser intensity rapidly tends to zero, the atom is left in the state $|F=1,m_F=+1\rangle_1$ and now can act as a receiving atom.

\subsection{Production of the output field state}
Here we analyze the output state of quantum field using Eqs.\eqref{eq:9}. The basis states of the sending system and outgoing photons are the atomic ground Zeeman states $|m_F\rangle$, vacuum state of the cavity mode $|0\rangle_{1c}$, and photonic states $|j\rangle$ with free propagating $j$ photons of frequency $\omega_c$, which are coupled to a single-mode optical fiber. The state $|j=2\rangle$ is not a $j$-Fock state, because two single-photon wave packets are in different temporal modes with wave functions $\Phi_i(t), i=1,2,$, which are found in Eqs.\eqref{eq:19}. The total state $|\Psi_1(t)\rangle$ can be then expanded in this basis as an entangled state between the atom and the outgoing light in the form
\begin{equation}
|\Psi_1(t)\rangle = \biggl (\sum_{m_F=-1}^{1}\sum_{j=0}^{m_F+1}\beta_{m_F,j}(t)|m_F\rangle_1|j\rangle\biggr )|0\rangle_{1c},\label{eq:11}
\end{equation}
where the coefficients $\beta_{m_F,j}(t)$ are normalized complex-valued amplitudes of the probabilities that at time $t$ the atom is in the state $|m_F\rangle_1$ and the number of photons in the resulting field is $j$. At $t\rightarrow -\infty$ the state $|\Psi_1(t)\rangle$ coincides with the initial state $|\Psi_{1,\text{in}}\rangle$ defined in Eq.\eqref{eq:4}. From this comparison, we find the initial values of $\beta_{-1,0}(-\infty)=c_{-1}$ and $\beta_{0,0}(-\infty)=c_{0}$, while the remaining coefficients are initially zero.

Our goal is to show that long after the interaction with the atom the state $|\Psi_1(t)\rangle$ is reduced to the final form
\begin{equation}
|\Psi_{1,\text{fin}}\rangle = |\Psi_1(\infty)\rangle = |+1\rangle_1|0\rangle_{1c} \otimes |\Psi_{\text {PNSS}}(t)\rangle,\label{eq:12}
\end{equation}
where the atom occupies the state $|m_F=+1\rangle$, while the output state of quantum field is the PNSS of two- and one-photon states
\begin{equation}
|\Psi_{\text {PNSS}}(t)\rangle=c_{-1}|1_{\Phi_1},1_{\Phi_2}\rangle + c_0 |1_{\Phi_1}\rangle.\label{eq:13}
\end{equation}
The coefficients $\beta_{m_F,j}(t)$ are connected to the populations of atomic states by the relation
\begin{equation}
\langle\sigma_{m_F}(t)\rangle = Tr[\rho_1(t)\sigma_{m_F}]=\sum_{j=0}^{m_F+1}|\beta_{m_F,j}(t)|^2,\label{eq:14}
\end{equation}
where $\rho_1(t)=|\Psi_1(t)\rangle \langle \Psi_1(t)|$.
Using Eqs.\eqref{eq:9}, $\beta_{m_F,j}(t)$ are found to be
\begin{subequations}
\begin{eqnarray}
& & \beta_{m_F=-1,j=0}(t)=c_{-1} e^{-\vartheta(t)/2},\label{eq:15a}\\
& & \beta_{m_F=0,j=0}(t)=c_0 e^{-\vartheta(t)/2},\label{eq:15b}\\
& & \beta_{m_F=0,j=1}(t)=c_{-1}[\vartheta(t) e^{-\vartheta(t)}]^{1/2},\label{eq:15c}\\
& & \beta_{m_F=1,j=0}(t)=0,\label{eq:15d} \\
& & \beta_{m_F=1,j=1}(t)=c_0 [1-e^{-\vartheta(t)}]^{1/2},\label{eq:15e}\\
& & \beta_{m_F=1,j=2}(t)=c_{-1}[1-(1+\vartheta(t))e^{-\vartheta(t)}]^{1/2},\label{eq:15f}
\end{eqnarray}\label{eq:15}
\end{subequations}
showing that at large times, when $\vartheta(t)e^{-\vartheta(t)}\ll1$, which is achieved at $kt\sim 3$, only two amplitudes stay on: $\beta_{m_F=1,j=1}(t\rightarrow\infty)=c_0$ and $\beta_{m_F=1,j=2}(t\rightarrow\infty)=c_{-1}$. Consequently, the state $|\Psi_1(t)\rangle$ is asymptotically transformed into $|\Psi_{1,\text{fin}}\rangle$ indicating that the quantum information encoded initially in the atomic superposition state $|\Psi_{1,\text{in}}\rangle$, Eq.\eqref{eq:4}, is completely converted into PNSS given by Eq.\eqref{eq:13}. Here it was assumed that no dephasing of photonic states occurs in the cavity mirror and communication channel.

Similarly, the photon distributions $P_j(t)$ in the resulting field, that is the population of the photonic state $|j\rangle$, is defined as the probability that the output field contains $j$ photons, no matter what state the atom is in, and, thereby, is given by the sum of $|\beta_{m_F,j}(t)|^2$ over all possible $m_F$
\begin{eqnarray} \label{solution}
P_{j}(t)= \sum_{m_F=-1}^1|\beta_{m_F,j}(t)|^2, \quad j=0,1,2. \label{eq:16}
\end{eqnarray}
$P_j(t)$ are calculated by means of Eqs.\eqref{eq:15} and are shown in Fig.\ref{fig:fig3} for the same parameters as in Fig.\ref{fig:fig2}. It is apparent that, as time increases, the states with $j=1,2$ remain populated as $|c_0|^2$ and $|c_{-1}|^2$, respectively, indicating the deterministic generation of PNSS.
\begin{figure}[h] \rotatebox{0}{\includegraphics*
[scale =0.7]{Fig3.eps}} \caption{(Color online) Dynamics of the photon number (indicated on the curves) distribution in the generated light for the same parameters as in Fig.\ref{fig:fig2}.
\label{fig:fig3}}
\end{figure}

Now we find the flux of produced photons, which is needed to calculate the wave functions of emitted photons. In units of photons per unit time, the flux of the outgoing photons is defined by
\begin{equation}
\frac{dn_{\text{out}}}{dt}(t) = \langle a^{\dag}_{1,\text{out}}(t)a_{1,\text{out}}(t)\rangle,\label{eq:17}
\end{equation}
which determines the shape of emitted intensity. Here $n_{\text{out}}(t)$ is the mean photon number in the time interval $(-\infty,t]$ of the output field $a_{1,\text{out}}(t)$ from the first cavity, which is obtained from input-output relation and Eq.\eqref{eq:5}. Then, using Eq.\eqref{eq:8}, we have
\begin{equation}
\frac{dn_{\text{out}}}{dt}(t)=\alpha_1f_1(t)\sum_{m_F=-1}^{0}\langle \sigma_{m_F}(t)\rangle=\alpha_1f_1(t)[1-\langle \sigma_1(t)\rangle].\label{eq:18}
\end{equation}
The total flux is obviously the sum of the fluxes or intensities of the first and second photon pulses, which are readily separated in Eq.\eqref{eq:18} by substituting $\langle \sigma_1(t)\rangle$ from Eq.\eqref{eq:9c} that yields
\begin{subequations}
\begin{eqnarray}
\frac{dn_{\text{I}}}{dt}(t) &=& |\Phi_1(t)|^2= \alpha_1f_1(t)e^{-\vartheta(t)},\label{eq:19a}\\
\frac{dn_{\text{II}}}{dt}(t) &=& |c_{-1}|^2|\Phi_2(t)|^2 \nonumber\\
&=& |c_{-1}|^2\alpha_1f_1(t)\vartheta(t)e^{-\vartheta(t)},\label{eq:19b}
\end{eqnarray}\label{eq:19}
\end{subequations}
where the wave functions of the photons $\Phi_{1,2}(t)$ are considered to be real taking into account that they have the same phase as the control field $\Omega_1$, which can be taken zero without loss of generality. The partial fluxes corresponding to the preceding dynamics shown in Fig.\ref{fig:fig3} are displayed in Fig.\ref{fig:fig4}. The first photon intensity does not  evidently depend  on the population distribution between atomic states, while the second photon is emitted only if $c_{-1}\neq 0$. In both cases, the photon temporal profile is easily controlled being proportional to the $\Omega_1$ laser pulse shape.

The mean photon number is obtained by integrating Eq.\eqref{eq:18} yielding to
\begin{equation}
n_{\text{out}}(t)=(1+|c_{-1}|^2)(1-e^{-\vartheta(t)})-|c_{-1}|^2\vartheta(t)e^{-\vartheta(t)},\label{eq:20}
\end{equation}
which coincides with $n_{\text {total}}=\sum_{j=1}^{2} jP_{j}(t)$, as expected. This equation shows that for small $\vartheta(t)$, the generation of one photon dominates, where $n_{\text{out}}(t)=\vartheta(t)$  increases proportionally to the pump energy confined in that time interval, while two-photon emission is manifested at larger times, as it grows quadratically in $\vartheta(t)$ as $|c_{-1}|^2\vartheta^2(t)/2$.

\begin{figure}[h] \rotatebox{0}{\includegraphics*
[scale =0.7]{Fig4.eps}} \caption{(Color online) Partial fluxes of the first and the second photons $dn_j/dt,j=\text{I,II}$ (indicated on the curves) for the same conditions as in Fig.\ref{fig:fig2}. The total flux is shown by the green line. The laser field profile is decreased by factor of two.}
\label{fig:fig4}
\end{figure}

Of particular importance is the question of joint generation of photons in the state $|1_{\Phi_1},1_{\Phi_2}\rangle$, which can be revealed by two photon correlation function at zero time delay
\begin{equation}
g^{(2)}(t) = \frac{\langle a_{\text{out}}^{\dagger 2}(t)a_{\text{out}}^2(t)\rangle}{\langle a_{\text{out}}^\dagger(t)a_{\text{out}}(t)\rangle^2}.\label{eq:21}
\end{equation}

Here $\langle a_{\text{out}}^\dagger(t)a_{\text{out}}(t)\rangle^2$ gives the probability of emitting two single photons independently, while $\langle a_{\text{out}}^{\dagger2}(t) a_{\text{out}}^2(t)\rangle$ represents the probability of the generation of paired photons. In Fig.\ref{fig:fig5} the photon correlation displays a small antibunching in the main region $-10\leq kt\leq -3$ of the photon generation, indicating the predominance of the generation of uncorrelated photons compared to joint generation of photons. Moreover, the requirement that the intensity of the emitted light calculated in terms of PNSS coincides with Eq.\eqref{eq:19}
\begin{align}
& &\langle \Psi_{\text {PNSS}}(t)|a_{\text{out}}^{\dagger}(t) a_{\text{out}}(t)|\Psi_{\text {PNSS}}(t)\rangle \nonumber \\
& &=|\Phi_1(t)|^2+|c_{-1}|^2|\Phi_2(t)|^2\label{eq:22}
\end{align}
is satisfied, if the states $|1_{\Phi_1}\rangle$ and $|1_{\Phi_2}\rangle$ are orthogonal: $\langle 1_{\Phi_1}|1_{\Phi_2}\rangle=0$. In this case, the operator $a_{1,\text{out}}(t)$ can be represented as \cite{20}
\begin{equation}
a_{1,\text{out}}(t) = \sum_i\Phi_i(t)\hat b_i, \label{eq:23}
\end{equation}
where the independent annihilation operators $\hat b_i$ destroy the single-photon states in the usual way by operation $\hat b_i|1_{\Phi_i}\rangle=|0_{\Phi_i}\rangle$ and have the standard boson commutation relations $[\hat b_i,\hat b^\dagger_j]=\delta_{ij}$.

\begin{figure}[h] \rotatebox{0}{\includegraphics*
[scale =0.7]{Fig5.eps}} \caption{(Color online) Second-order correlation function of generated photons at zero time delay for the same parameters as in Fig.\ref{fig:fig2}}
\label{fig:fig5}
\end{figure}

\section{\protect\normalsize PNSS STORAGE IN THE RECEIVING NODE}
In the receiving node, the atom with the same level configuration is initially prepared in the state $|F=1,m_F=1\rangle_2$ and the cavity field is in the vacuum. Assuming that the losses in the communication channel are effectively switched off, the PNSS generated from the sending cavity constitutes the input field for the receiving one, thus the initial state of receiving system is given by
\begin{equation}
|\Psi_{2,\text{in}}\rangle = |+1\rangle_2 |0\rangle_{2c}\biggl (c_{-1}|1_{\Phi_1},1_{\Phi_2}\rangle + c_0 |1_{\Phi_1}\rangle\biggr ).\label{eq:24}
\end{equation}

The atom interacts with the $\sigma^+$ polarized laser field of frequency $\omega$ and the peak Rabi frequency $\Omega_2$, which can be different from $\Omega_1$. The laser field is switched on shortly before the arrival of the photons, in order to avoid the atomic decay from the upper level $|F'=2,m_F'=+2\rangle_2$ into the states outside of the system during the PNSS storage. Similarly, the same magnetic field as in the sending system is applied to provide two-photon resonant Raman transition with linearly polarized cavity photons.

The complete conversion of PNSS into the superposition of ground Zeeman states of the receiving atom implies that the output quantum field from the second cavity is identically zero at all times. This amounts to formally setting $a_{2,\text{out}}(t)=0$ in the input-output relation $a_{2,\text{out}}(t)-a_{2,\text{in}}(t)=\sqrt{k}a_2(t)$ for the second cavity. Then, using $a_{2,\text{in}}(t)=a_{1,\text{out}}(t-\tau)$, we have
\begin{equation}
a_2(t) = -\frac{1}{\sqrt{k}}a_{1,\text{out}}(t-\tau),\label{eq:25}
\end{equation}
where $\tau$ represents the time for the photons to travel from one cavity to the other. We can eliminate $\tau$ according to the formalism of cascaded quantum systems \cite{18,19}, which include also our scheme, thereby $\tau$ can be omitted in what follows.

\subsection{Evidence of PNSS storage from conservation laws}
Here we derive the conservation law for the numbers of photons and atomic excitations. The effective interaction Hamiltonian for the receiving system has the form similar to Eq.\eqref{eq:3}
\begin{equation}
H=\hbar G_2 f_2^{1/2}(t) \biggl (a_2^{\dag}(t)(\varrho_{1,0}+\varrho_{0,-1})+(\varrho_{0,1}+\varrho_{-1,0})a_2(t)\biggr ),\label{eq:26}
\end{equation}
where $\varrho_{i,j} = |m_F=i\rangle_{22}\langle m_F=j |$ are the operators of the receiving atom, $G_2=g\Omega_2/\Delta$ and $f_2(t)$ is the second laser intensity shape. In the absence of relaxations, the equations for the photon number $a_2^{\dag}a_2$ and atomic population operators $\varrho_{i,i}(t)\equiv\varrho_i(t), i=0,-1,$ in the second cavity are obtained in the form
\begin{widetext}
\begin{subequations}
\begin{eqnarray}
& & \frac{d(a_2^{\dag}a_2)}{dt}(t) =-i k G_2\biggl [a_2^{\dag}(\varrho_{1,0}+\varrho_{0,-1}) -(\varrho_{0,1}+\varrho_{-1,0})a_2\biggr ]+k a_2^{\dag}a_2,\label{eq:27a}\\
& & \frac{d\varrho_0}{dt}(t)=i G_2\biggl(a_2^{\dag}(\varrho_{1,0}-\varrho_{0,-1})+(\varrho_{-1,0}-\varrho_{0,1})a_2\biggr),\label{eq:27b}\\
& & \frac{d\varrho_{-1}}{dt}(t)=i G_2(a_2^{\dag}\varrho_{0,-1}-\varrho_{-1,0}a_2)\label{eq:27c}.
\end{eqnarray}\label{eq:eq27}
\end{subequations}
\end{widetext}
By combining and integrating these equations and using Eq.\eqref{eq:25}, we derive the conservation law
\begin{equation}
N_0(t)+2N_{-1}(t)=n_{\text{out}}-\frac{1}{k}{\mathcal F}(t),\label{eq:28}
\end{equation}
where $N_{0(-1)}$ is the population of ground state Zeeman sublevel $m_F=0(-1)$ of the receiving atom, ${\mathcal F}(t)=\langle a^{\dag}_{1,\text{out}}(t)a_{1,\text{out}}(t)\rangle$ is the flux of outgoing photons from the sending cavity, and $n_{\text{out}}=\int \limits_{-\infty}^t{\mathcal F}(t')dt'$ is defined in Eq.\ref{eq:17}. From Eq.\eqref{eq:28} we recognize that $N_0(-\infty)=N_{-1}(-\infty)=0$, i.e. the receiving atom is initially in the state $|F=1,m_F=1\rangle_2$. For large times, taking into account that $N_1(\infty)=0$ and the photon number tends to $n_{\text{out}}(\infty)=1+|c_{-1}|^2$ following from Eq.\eqref{eq:20}, while $F(\infty)\rightarrow 0$, we find $N_{-1}(\infty)=|c_{-1}|^2$ and $N_0(\infty)=|c_0|^2$. This demonstrates that the sending and receiving atoms ultimately exchange initial states, thus implementing the complete transfer of the quantum information between the two network nodes. The Zeeman coherence for the receiving atom is next shown by analytical calculations of the population amplitudes with simultaneous determination of the second laser pulse shape.

\subsection{Coherent absorption of photons. Tuning of the laser pulse shape }
We expand the state of the receiving system as
\begin{equation}
|\Psi_2(t)\rangle = \biggl (\sum_{m_F=-1}^{1}\sum_{j=0}^{m_F+1}\gamma_{m_F,j}(t)|m_F\rangle_2|j\rangle\biggr ),\label{eq:29}
\end{equation}
where, similar to $\beta_{m_F,j}(t)$ in Eq.\eqref{eq:11}, $\gamma_{m_F,j}(t)$ are normalized amplitudes of the probabilities that at time $t$ the receiving atom is in the state $|m_F\rangle_2$ and the number of incoming photons is $j$. The level populations of the second atom are calculated by the formula
\begin{equation}
\langle\varrho_{m_F}(t)\rangle = \sum_{j=0}^{m_F+1}|\gamma_{m_F,j}(t)|^2.\label{eq:30}
\end{equation}
We find the coefficients $\gamma_{m_F,j}(t)$ from the Schr\"odinger equation for $|\Psi_2(t)\rangle$ with the use of Hamiltonian \eqref{eq:26}, where the operator $a_2(t)$ is replaced by $a_{1,\text{out}}(t)$ from Eq.\eqref{eq:25}. It should  be taken into account that the photonic state in the $\gamma_{m_F=0,j=1}$ term is the superposition of two one-photon states: $|j=1\rangle=\frac{1}{\sqrt{2}}(|1_{\Phi_1},0_{\Phi_2}\rangle+|0_{\Phi_1},1_{\Phi_2}\rangle)$. Then, by introducing new variables
\begin{subequations}
\begin{eqnarray}
& & \eta(t) = 2\frac{|G_2|}{\sqrt{k}}\int \limits_{-\infty}^tf_2^{1/2}(\tau)\Phi_1(\tau)d\tau,\label{eq:31a}\\
& & \zeta(t) = \frac{|G_2|}{\sqrt{k}}\int \limits_{-\infty}^tf_2^{1/2}(\tau)\biggl(\Phi_1(\tau)+\Phi_2(\tau)\biggr)d\tau\label{eq:31b}
\end{eqnarray}
\end{subequations}
and using Eq.\eqref{eq:23}, the equations for $\gamma_{m_F,j}(t)$ are derived in a simple form
\begin{subequations}
\begin{eqnarray}
\frac{d\gamma_{ 0,0}(t)}{d\eta} = \frac{i}{2}\gamma_{1,1}(t)e^{-i\varphi_2},\label{eq:32a}\\
\frac{d\gamma_{1,1}(t)}{d\eta} = \frac{i}{2}\gamma_{0,0}(t)e^{i\varphi_2}\label{eq:32b}
\end{eqnarray}\label{eq:32}
\end{subequations}
and
\begin{subequations}
\begin{eqnarray}
\frac{d\gamma_{-1,0}(t)}{d\zeta} = \frac{i}{\sqrt{2}}\gamma_{0,1}(t)e^{-i\varphi_2},\label{eq:33a}\\
\frac{d\gamma_{0,1}(t)}{d\zeta} = \frac{i}{\sqrt{2}}\biggl(\gamma_{1,2}(t)e^{-i\varphi_2}+\gamma_{-1,0}(t)e^{i\varphi_2}\biggr),\label{eq:33b}\\
\frac{d\gamma_{ 1,2}(t)}{d\zeta} = \frac{i}{\sqrt{2}}\gamma_{0,1}(t)e^{i\varphi_2}.\label{eq:33c}\nonumber
\end{eqnarray}\label{eq:33}
\end{subequations}
where $\varphi_2$ is the phase of $\Omega_2$ field. These equations describe the coherent excitation of two-level and three-level systems by "one- and two-photon" absorption, respectively, where the role of the "one-photon transition" in the first case is played by the first Raman transition $|F=1,m_F=1\rangle_2\rightarrow |F=1,m_F=0\rangle_2$ in Fig.\ref{fig:fig1} (right) with the effective pulse area $\eta(t)$. In the second case, the "two-photon excitation" is accomplished by the double Raman transition $|F=1,m_F=1\rangle_2\rightarrow |F=1,m_F=0\rangle_2\rightarrow |F=1,m_F=-1\rangle_2$ with total pulse area $\zeta(t)$.

Solving the Eqs.\eqref{eq:32} and \eqref{eq:33} subject to the initial conditions $\gamma_{1,2}(-\infty)=c_{-1}$ and $\gamma_{1,1}(-\infty)=c_0$ following from Eq.\eqref{eq:24}, we get for $\varphi_2=\pi/2$
\begin{equation}
\gamma_{0,0}(t) = c_0\sin[\eta(t)/2], \quad \gamma_{1,1}(t) = c_0\cos[\eta(t)/2]\label{eq:34}
\end{equation}
and
\begin{subequations}
\begin{eqnarray}
\gamma_{1,2}(t) = \frac{1}{2}c_{-1}\biggl [1+\cos\zeta(t)\biggr],\label{eq:35a}\\
\gamma_{0,1}(t)=\frac{1}{\sqrt{2}}c_{-1}\sin\zeta(t),\label{eq:35b}\\
\gamma_{-1,0}(t) = \frac{1}{2}c_{-1}\biggl [1-\cos\zeta(t)\biggr].\label{eq:35c}
\end{eqnarray}\label{eq:35}
\end{subequations}
It is evident that the complete mapping of photons onto the atomic ground states can be achieved by means of effective two-photon (Raman) $\pi$-pulses, which imposes the following  conditions on the pulse areas
\begin{equation}
\eta(\infty)=\zeta(\infty)=\pi,\label{eq:36}
\end{equation}
leading to $\gamma_{0,0}(\infty)=c_0$ and $\gamma_{-1,0}(\infty)=c_{-1}$ and zero for the remaining coefficients. As a result, the second atom is settled in the final state
\begin{equation}
|\Psi_{\text{2,fin}}\rangle=c_{-1} |-1\rangle_2 + c_0 |0\rangle_2,\label{eq:37}
\end{equation}
which coincides in form with the initial state of the sending atom in Eq.\eqref{eq:4}. It is obvious that the fidelity of the state $|\Psi_{\text{2,fin}}\rangle$ with $|\Psi_{\text{1,in}}\rangle$, which have commuting density matrices, is equal to unity. The populations of ground Zeeman sublevels of the second atom found from Eq.\eqref{eq:30} are displayed in Fig.\ref{fig:fig6}.

The strength and temporal shape of $\Omega_2(t)$ pulse is fully determined by the conditions \eqref{eq:36}. For the used parameters, the latter are well fitted by Gaussian pulse with $\Omega_2=\Omega_1$ and duration $T_2\sim1~\mu$s. The time evolution of $\eta(t)$ and $\zeta(t)$ is shown in Fig.\ref{fig:fig7}. It should be noted that for the transfer of atomic quantum state, our scheme does not require time-symmetric photonic wave packets, in contrast to the scheme proposed in Ref.\cite{2}. The coherent absorption of arbitrarily shaped traveling photons in the second cavity is governed by the area of two-photon Raman pulses, where the time dependence of the second control field is appropriately adapted.
\begin{figure}[t] \rotatebox{0}{\includegraphics*
[scale =0.7]{Fig6.eps}} \caption{(Color online) Evolution of the populations of ground Zeeman states $|m_F=-1\rangle_1$ (red), $|m_F=0\rangle_1$ (blue) and $|m_F=+1\rangle_1$ (black) of the second atom for the $\Omega_2 = \Omega_1$ Gaussian laser pulse of intensity profile $f_2(t)=e^{-(t/T_2)^2}$ with duration $T_2=1~\mu$s. The profiles of the laser fields in the first and second cavities are shown by the red and blue dotted lines, respectively. For the sending system, the same parameters as in Fig.\ref{fig:fig2} are used.
\label{fig:fig6}}
\end{figure}

\begin{figure}[t] \rotatebox{0}{\includegraphics*
[scale =0.7]{Fig7.eps}} \caption{(Color online) Variables $\eta(t)$(red) and $\zeta(t)$(blue) as functions of time for the same parameters as in Fig.\ref{fig:fig6}.
\label{fig:fig7}}
\end{figure}

\subsection{Quantum state transfer via photonic qutrit}

The most important feature of multiphoton states is their ability to carry more information than a photonic qubit. One way to increase the information content of PNSS is to include into the superposition the states with more than two photons, which will allow to send information with increased capacity parameters. However, the current technologies do not support these statement, since along with the increase of the photon number, the losses in the communication channel increase exponentially. In contrary to this, our protocol is capable of producing a photonic qutrit without increasing the number of photons we use and, thus, preserving the robustness and efficiency of the PNSS qubit discussed in the next section. To this end, the atom is initially prepared in the superposition of the Zeeman sublevels $m_F=-1,0,+1$ in the sending node. Obviously, after interacting of the atom with the $\Omega_1(t)$ field, the generated photon state leaving the first cavity is analogous to the state \eqref{eq:13} and has the form
\begin{equation}
|\Psi_{\text {PNSS}}(t)\rangle=c_{-1}(t)|1_{\Phi_1},1_{\Phi_2}\rangle + c_0(t) |1_{\Phi_1}\rangle + c_{+1}(t)|0\rangle,\label{eq:13prime}
\end{equation}
where the coefficients $c_{-1},c_0,c_{+1}$ are the population amplitudes of the Zeeman sublevels  $m_F=-1,0,+1$, respectively, and all of them differ from $0$ at the initial time moment $t=-\infty$. Thus, the atom qutrit state is completely mapped into the photonic qutrit state. Using the same method, the state \eqref{eq:13prime} is transferred to the receiving atom, which is initially prepared at the Zeeman sublevel $m_F=+1$. Similar to the case of the qubit transfer, the second atom coherently absorbs the photons and  passes into the superposition state  of three ground-state Zeeman sublevels, which coincides in form with the initial state of the first atom.

\section{\protect\normalsize DISCUSSIONS}
At short communication distances, where the photon losses are negligible, the presented protocol is fully deterministic, relied on the high signal-to-noise ratio Eq.\eqref{eq:6} and enhanced Raman emission of linearly polarized cavity photons in the sending node and their controlled coherent absorption in the receiving system. An important advantage of the present scheme is the capability of multi-photon superposition states to transmit an incomparably greater information than is possible with a single-photon transfer. Imperfections of the scheme are manifested at large transmission distances caused by photon losses. Presently, the photon losses are comprehensively analyzed in \cite{Q} for two protocols of deterministic QST based on wave packet shaping \cite{2} and adiabatic passage \cite{P}. Remind that in the first case, the state transfer is realized by producing a time-symmetric photon wave packet inside a fiber and in the second one the QST is accomplished by performing the adiabatic passage with classical driving fields in a counterintuitive order. This analysis has shown that the state transfer by adiabatic passage can mitigate the effects of cavity losses, while the fiber transmission losses cannot be overcome using either of the two methods. Our approach does not fit into this paradigm, as we do not use the time-symmetric photon wave packets, and the control field in the receiving node is delayed with respect to the control field in the sending node. Nevertheless, our findings are analogous to those presented in \cite{Q}, demonstrating that the cavity losses can be strongly suppressed by making the signal-to-noise ratio sufficiently large, as shown in Sec.IIB, but due to fiber losses the QST is strictly limited by Eq.\eqref{eq:38} given below.

To show this we evaluate the efficiency of the QST by introducing the success probability as
\begin{equation}
P_{j,\text{trans}}=p_{j,\text{em}}\eta_{j,\text{trans}}p_{j,\text{abs}},\label{eq:38}
\end{equation}
with $j=1,2$ defined as the product of quantum-mechanical probabilities $p_{j,\text {em}}$ and $p_{j,\text {abs}}$ of $j$ photon emission in the sending and their absorption in the receiving nodes, respectively, by the transmission efficiency $\eta_{j,\text{trans}}=\text{exp}(-\frac{jL_0}{L_{\text{att}}})$, where $L_0$ is the distance between the nodes and $L_{\text{att}}$ is the communication channel attenuation length \cite{21}. It is apparent that the two-photon transmission efficiency is quadratically smaller compared to the one photon case: $\eta_{2,t}=\eta_{1,t}^2$. Today, the commercial fibers feature an attenuation of 2~dB/km at 800~nm \cite{21}, which corresponds to $L_{\text{att}}=2.2$~km. This means that in the present scheme with $p_{j,\text {em}}=p_{j,\text {abs}}\sim 1$ the success probability of PNSS transfer between the nodes connected by an optical fiber link of 60~m length, as in the experiment \cite{3}, is unity. At larger distances $L_0\sim L_{\text{att}}$, the efficiency of two-photon transfer decreases in our scheme by approximately an order of magnitude. However, it remains comparable with the efficiency of an ideal transfer of a single-photon polarization state in the scheme of Ref.\cite{3}, if one takes into account that in that scheme the probability $p_{1,\text {em}}$ of this state generation in the sending node is limited by the value of $25\%$. Nevertheless, as at these distances the fidelity of the state transfer process becomes dependent on its efficiency, a possible way to overcome this difficulty is to filter out successful events by a heralding signal. This is comparatively easy to implement for the creation of remote atom-atom entanglement, as evidenced by a large number of publications on this issue (see, for example, \cite{21}). As to the heralded QST, to our best knowledge, so far only one protocol has been proposed and realized for a heralded, high-fidelity mapping of the polarization state of a single photon onto an atomic qubit using Zeeman manifolds of two different atomic states \cite{E,kurz,F}. It is worth noting that the extended version of this scheme has been used in \cite{R} to entangle partner photons absorbed by ions in remote traps. At the same time, such an approach is not yet available in the case of multiphoton absorption, therefore the implementation of heralding remains challenging with our protocol. However, as suggested in \cite{3}, the successful storage of incoming photons in the second cavity can be verified by analyzing the Zeeman state populations of the second atom using the cavity-assisted fluorescence detection \cite{B,S,T}.

The superposition state architectures require that the phase acquired by photons in long fiber links must remain constant for times larger than the travel time. In this sense, the phase stabilization is a common problem and requires an identical solution in all protocols. In our scheme, two photons in PNSS, which are not correlated or entangled, have the same polarization, and suffer from the same losses and same polarization and velocity fluctuations, especially as they are efficiently outcoupled into a single-mode optical fiber with almost overlapped temporal profiles. Therefore, if only phase noise in optical fibers is considered, the two-photon state undergoes only an overall phase change, which can deteriorate the PNSS fidelity. However, in conventional conditions, the mean phase shift due to the fluctuations in fibers is about $0.1$~rad/km \cite{noise}, which is small enough to neglect the phase noise at distances where the photon losses start. This is also witnessed by the large values of the fidelity reaching 85\% for the transferred photonic polarization state in the experiment of Ref.\cite{3}. Moreover, as shown in \cite{U}, the width of the Gaussian distribution of the phase noise in the Mach-Zehnder interferometer is even lower, so that the phase remains constant for several tens of kilometers.

We conclude our discussion by returning to the well-studied question that the atomic motion in the cavity can be significantly affected by photon recoil from emission and absorption of even a single photon, which can no longer be ignored in the case of multiphoton processes. To remove this effect, for example in a photon emission, the atomic recoil $L_\text{rec}$ has to be made negligible with respect to the photon wavelength $\lambda$, where  $L_\text{rec}$ is calculated as the distance the atom travels during the time interval $T_\text{phot}$ between two time moments of the first and second photons emission: $L_\text{rec}=\hbar kT_\text{phot}/m$, where $m$ is the atomic mass, $k=2\pi/\lambda$. Since $T_\text{phot}$ is  reciprocal to the generation rate of photons in the cavity, $T_\text{phot}^{-1}\sim G_1=g\Omega_1/\Delta$, then from $L_\text{rec}\ll \lambda$ one finds $\omega_\text{rec}\ll G_1$, where $\omega_\text{rec}=\hbar k^2/2m$ is the recoil frequency associated with the kinetic energy transfer to the atom in a single photon scattering event. Usually, to localize the atom at the center of the cavity mode,  high-intensity laser beams along all three directions are used thus reducing the recoil frequency to about 4 kHz \cite{V}.  We assume that this is the case in our model, where $G_1\simeq 1.5$~MHz, so that the cavity emission does not change the motional state of the atom. This is true for the photon absorption in the second cavity as well.

 These observations show that to suppress the  environmental effects no additional efforts are needed in our scheme, while its advantages are obvious.

\section{\protect\normalsize CONCLUSION}
In conclusion, we have proposed and analyzed a robust and efficient scheme for deterministic transfer of quantum states between two remote cavity-trapped atoms by means of traveling photon-number superposition states.The quantum information encoded in ground Zeeman sublevels of the first atom is released in the photonic qubit or qutrit, depending on the number of superposed Zeeman states, via cavity-assisted Raman scattering and upon reaching the second atom is stored in the ground Zeeman states of the latter via coherent absorption of photons. We have demonstrated that our scheme allows reliable overall transfer of quantum information at the distances, where the photon losses are negligible, without using a quantum error correction.
At the same time, our scheme displays no less reliable protection against the propagation losses at large distances as compared to previous protocols with a single photon transfer.

These results promise also a successful distribution of entanglement between distant nodes in quantum networks. This study is currently under way.

\subsection*{Acknowledgments}

Authors thank to S. Gu\'erin and A. Kuhn for helpful discussions and comments. This research has been conducted in the scope of the International Associated Laboratory (CNRS-France $\&$ SCS-Armenia)  IRMAS. We acknowledge additional support from the Science Basic Foundation of the Government of the Republic of Armenia.

redpajama_set_name: RedPajamaArXiv


text:
An arş (Ottoman Turkish آرش) is an old Turkish unit of length.

The word means 'forearm' and thus the measure corresponds to a cubit.

See also

 arşın, the Ottoman yard

Notes

Obsolete units of measurement
Units of length
Ottoman units of measurement

redpajama_set_name: RedPajamaWikipedia


text:
Interpretations and Actions: February 2010
Vol. 23, No. 2
Community Development Investment Letters
2009-6 (PDF) Investment in Fund to Install Photovoltaic System in Low income Housing Tax Credit Project - A national bank may make an investment in a Community and Economic Development Entity that will install photovoltaic systems in low-income housing tax credit projects. These systems will qualify for renewable energy tax credits. 01/06/2009
Corporate Decisions
2010-01 (PDF) Application by the Federal Deposit Insurance Corporation (FDIC) to charter a new national bank with the title of "Deposit Insurance National Bank of New Baltimore", under 12 USC 1821(m), to assume the insured deposits of Citizens State Bank, New Baltimore, Michigan, an insured bank in default, and to perform other activities (Control Number 2009-CE-02-043), 12/18/2009
2010-02 (PDF) Application by The Huntington National Bank, Columbus, Ohio, to establish six temporary branches in Michigan to assist the Federal Deposit Insurance Corporation (FDIC) in its resolution of Citizens State Bank, New Baltimore, Michigan, a state-chartered bank that was closed by the Michigan state regulators on December 18, 2009 and placed into receivership (Control Numbers 2009-CE-05-190 thru 195), 12/18/2009
2010-03 (PDF) Application by the Federal Deposit Insurance Corporation (FDIC) to charter a new national bank with the title of "Deposit Insurance National Bank of Kaysville", under 12 USC 1821(m), to assume the insured deposits of Barnes Banking Company, Kaysville, Utah, an insured bank in default, and to perform other activities (Control Number 2010-WO-01-0001), 01/15/2010
2010-04 (PDF) Application by Zions First National Bank, Salt Lake City, Utah, to establish ten temporary branches in Utah to assist the Federal Deposit Insurance Corporation (FDIC) in its resolution of Barnes Banking Company, Kaysville, Utah, a state-chartered bank that was closed by the Utah state regulators on January 15, 2010 and placed into receivership (Control Numbers 2010-WE-05-0001 thru 0010), 01/15/2010
2010-05 (PDF) Acquisition by SCBT, National Association, Orangeburg, South Carolina, of assets and liabilities from Community Bank & Trust, Cornelia, Georgia ("Failed Entity") (Control Number 2010-NE-02-003), 01/29/2010
2010-06 (PDF) Application by Sunflower Bank, National Association, Salina, Kansas, to acquire from the Federal Deposit Insurance Corporation ("FDIC") as receiver, the deposits and certain assets of Bank of Leeton, Leeton, Missouri (Control Number 2010-WE-02-0001), 01/22/2010
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941 (PDF) Application to merge Wachovia Bank, National Association, Charlotte, North Carolina and Wachovia Bank of Delaware, National Association, Wilmington, Delaware with and into Wells Fargo Bank, National Association, Sioux Falls, South Dakota (Control Number 2009 ML 02 0012), 11/24/2009
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945 (PDF) Application by Premier American Bank, National Association, to acquire from the Federal Deposit Insurance Corporation as Receiver certain assets and liabilities of Florida Community Bank, Immokalee, Florida (Control Number 2010 WO 02 0003), 01/29/2010
Final Enforcement Actions
Enclosed is a copy of the OCC's news release number 2010-18, announcing the availability of enforcement actions. Copies of the final actions are available by writing to the OCC, Communications Division, Mail Stop 2-3, Washington, D.C. 20219. You may also submit your request electronically through the OCC's online FOIA site or fax your request to (202)-874-5274. When ordering, specify the appropriate enforcement action number.
Community Reinvestment Act (CRA) Performance Evaluations
Enclosed is a list of CRA performance evaluations that became public during the period of January 15, 2010 through February 14, 2010.
PLEASE NOTE: Interpretive Letters and No-Objection Letters reflect the views of the Comptroller's legal staff. Corporate Decisions, CRA Decisions and Conditional Approvals are from the office of Licensing Activities. The Community Development Investment Letters are from the office of Community Affairs. The list of CRA Ratings is from the Communications Division. For copies of the CRA evaluations, you may either contact the bank directly, or you may write to the Office of the Comptroller of the Currency (OCC) in any of three ways: by mail to the OCC, Attn: Communications Division, Mail Stop 2-3, Washington, D.C. 20219; by fax to (202) 874-5274; or electronically at the OCC's online FOIA site. You may also write to the OCC for copies of enforcement actions and charters with standard conditions.
Members of the news media are encouraged to cite the letter number when reporting or summarizing documents from this package. This helps us to process single requests based upon your citation in a timelier manner.
The Office of the Comptroller of the Currency publishes INTERPRETATIONS AND ACTIONS monthly. Subscriptions are available at a rate of $200 per year by writing to the Comptroller of the Currency, ATTN: Financial Management, Accounts Receivable, Mail Stop FM-2, Washington, DC 20219. Prepayment is requested. Suggestions, comments or questions may be sent to Jacqueline J. England, Comptroller of the Currency, Communications Division, Mail Stop 2-3, Washington, DC 20219.

redpajama_set_name: RedPajamaCommonCrawl


Get a print subscription to Reader's Digest and immediately enjoy free digital entry on any gadget. This intense amount of customisation can have you spending hours in your resort as you go from a single room to an island full of volleyball courts and excessive profile rooms with all of the luxuries you may ever want a resort. The Wildlife Park Sequence is a set of administration and building simulation games with many similarities to Zoo Tycoon. You are put in charge of a wildlife park and required to take care of the finances and guests that enter your park. The sport has massive enchantment to animal lovers, because it features over 60 completely different animal species.
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While the gameplay does sound enjoyable, it turns into even higher once you realise that you have a task to play in every (and I imply each) single element of the game. You need to not only create the studio (like building a house in The Sims) but also look after the careers of the film stars by ensuring they are spending their time properly. In the event that they feel like life is getting too annoying, they'll go off the rails similar to real actors do.
through monsterhigh.wikia.comIf you have heard of Mattel's Monster High , an American fashion-doll franchise impressed by horror and sci-fi/thriller flicks, you may be questioning why it is on this list. Well, the very fact is, Tynker tinkered with it and created a positive on-line gaming experience that ladies who already have a penchant for style-dolls can easily slide into—in truth, the draw used on Tynker's website is: Learn to Code with Monster Excessive Using the Tynker tools, a lady may create her personal dance celebration or scavenger hunt—as long as she codes it.
Our backyard shed was all the time full. Garden tools and the lawnmower stuffed one aspect and toys and dressing up clothes have been down the opposite aspect. We liked dressing up. Our field of garments was great for imaginary play. There have been scarves, hats, fans, clothes, skirts, web curtains, handbags, excessive heel sneakers, necklaces, nurse sets, cowgirl outfits, clown units and more.


Olapic is a Visual Commerce platform that tells your brand's story with curated customer photos & videos, helping you to improve the shopping experience and increase sales.
Olapic has been selected by Walmart to help suppliers curate and activate UGC and influencer content for its Connected Content Partner Program.
Olapic today introduced a number of new features to the Content in Motion™ platform to drive customer engagement, conversions and brand awareness.
As more money continues to be poured into startups, we're starting to see a growing number of venture capital firms and funds emerge that are increasingly..
New investment pours in as Pinterest inches closer to making the real world shoppable.
Why Nudge.ai? Reach out to the decision makers at Olapic with a personalized email - let them know that you found their recent news mention interesting.
Nudge.ai's relationship intelligence platform can help you find the right executive to reach out to at Olapic, such as Pau Sabria, Co-Founder, or Rachel Meranus, Chief Marketing Officer. Then get in touch and start a conversation.
Executives can be difficult to reach, but every company has connectors who bring together people and ideas. At Olapic, people like Bill Connolly, and Pau Sabria are likely connectors.
When Olapic is mentioned in the news, Nudge.ai often sees topics like Marketing, and Social Media. If your conversation focuses on these topics, you'll probably get Olapic's attention.
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Who in your network can introduce you to Olapic? Nudge.ai finds the best pathway to reach contacts at this company.


Although I wouldn't really know why you would like to use these features, they are provided for ISO compliance.
Define that term input (see read_term/3) maps each character read as CharIn to the character CharOut. Character conversion is only executed if the Prolog flag char_conversion is set to true and not inside quoted atoms or strings. The initial table maps each character onto itself. See also current_char_conversion/2.
Queries the current character conversion table. See char_conversion/2 for details.


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Home » Blog » Researchers link gene mutation to severe form of MS
Researchers link gene mutation to severe form of MS
June 3, 2016 Providence Health Team
Canadian researchers have found a genetic mutation linked to a severe and progressive form of MS, and they hope their work helps in the search for treatments for the disease.
Researchers from the University of British Columbia focused on two unrelated Canadian families to see whether members of each shared genetic consistencies that could account for MS, an unpredictable disease in which the immune system attacks the central nervous system.
In diagnosing MS, doctors use MRI to look for lesions on the brain and spinal cord that can lead to vision, memory and thinking problems. People with MS also can lose their ability to walk due to balance and coordination problems, and stiffness.
'At the edge of a cliff'
The researchers found that seven people from the families they studied carried a mutation to the gene NR1H3, which helps regulate inflammation:
In one family, five members carried the gene mutation and had primary-progressive MS. A second family had two relatives with the mutation and primary-progressive MS. Three more relatives carried the genetic mutation but had not been diagnosed with MS at the time of the study.
"This mutation puts these people at the edge of a cliff, but something still has to give them the push to set the disease process in motion," said the study's senior author, Carles Vilarino-Guell, an assistant professor of medical genetics and a member of the Djavad Mowafaghian Centre for Brain Health.
Poor prognosis
Close to 15 percent of MS patients develop the severe form of the disease. The Canadian researchers believe that people who carry the gene mutation have at least a 66 percent chance of developing the severe form of MS.
"If you have this gene, chances are you will develop MS and rapidly deteriorate," said study co-author Anthony Traboulsee, M.D., the MS Society of Canada research chair at UBC and director of Vancouver Coastal Health's MS and Neuromyelitis Optica Clinic. "This could give us a critical early window of opportunity to throw everything at the disease, to try to stop it or slow it. Until now, we didn't have much basis for doing that."
Read more about the study here.
Causes of MS
In addition to genetics, four other factors have been linked to MS:
Lower levels of vitamin D: Many researchers believe vitamin D may help regulate the immune system and reduce the risk of MS. People who live near the equator, where sunlight – which helps the body produce vitamin D – is plentiful, show a much lower risk of the disease than people in more temperate areas in the U.S.
Smoking: Numerous studies have found that smokers develop MS more often than non-smokers, and tend to have more brain lesions and brain shrinkage.
Infectious factors and viruses: Epstein Barr virus, usually associated with mononucleosis, has been consistently linked to the development of MS.
Autoimmune and inflammatory processes: Studies have suggested that MS can develop when regulation of the immune system breaks down.
Symptoms of MS
The National Institutes of Health divides symptoms for multiple sclerosis into two categories: initial and late-stage.
Initial symptoms include:
Vision problems such as blurred or double vision
Weak, stiff muscles, often with painful muscle spasms
Tingling or numbness in the arms, legs, trunk or face
Clumsiness and difficulty with balance when walking
Bladder-control problems
Dizziness that will not go away
Late-stage symptoms include:
Mental or physical fatigue
Mood changes such as depression or euphoria
Changes in the ability to concentrate or to multitask effectively
Difficulty making decisions, planning or prioritizing at work or in private life
Visit the National Multiple Sclerosis Society to learn more about MS, which affects 2.3 million people worldwide.
If you suspect that you may have symptoms of MS, talk to your health care provider about a full evaluation. You can find a Providence provider here.
Migraines in women could be linked to heart disease
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Child's play: Tips for buying safe and healthy toys
Have a fun, festive and memorable holiday season with a few simple toy-buying tips for the kids on your gift list.


Alpha Industries - Alpha Foundation For The Youth Inc.
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85% of our urban youth graduate high school with no real life skills, or able to obtain employment other than fast food industry jobs. Why? Most public school systems across the country stop offering these skilled trade basic introduction courses due to funding. There are certain industries that are finding it hard to fill their workforce when they experience a lot of retirement. These are good paying industries that will allow someone to raise a family.
The American criminal justice system holds more than 2.3 million people in 1,719 state prisons, 102 federal prisons, 942 juvenile correctional facilities, 3,283 local jails, and 79 Indian Country jails as well as in military prisons, immigration detention facilities, civil commitment centers, and prisons in the U.S. territories.


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Cell Phone Vibrator Motor Rpm
Lovense Remote-Controlled Sex Toys and Apps
Lovense is a Singapore-based sex tech company that makes remote-controlled sex toys, as well as software. The company is aimed at making it easier for people to feel pleasure. The company's products are designed for both men and women. Their remote-controlled toys come with many features such as:
Lovense sexual toys are extremely advanced and fun. With their unique syncing features that mimic the movements of your partner, even if you're hundreds of miles apart. The app allows you to sync your toys to your music library, so you can design your own rhythms and patterns.
Made from ABS and silicone plastic Lovense sexual toys can be safe for you and your family. They also feature the smoothest, highest-quality silicone. The sex toys can fit comfortably between a woman's feet and is designed to provide her a sexually enthralling experience while she strokes.
The Lovense toys for sex use Bluetooth technology to deliver the most intense pleasure. It is possible to connect your devices to a third-party app that allows your companion to manage the devices simultaneously. This technology allows you to simulate the sensation of real sexual sex without the risk of touching.
The Lovense Lush 3 sex toy is small and light and measures around three inches long. It features an insertable bulbous part which provides an intense stimulation. The tail is textured and comes with an ordinary c-shape that allows you to feel stronger vibrations than other devices.
If you're in search of an sex toys with remote controls that is just as entertaining as it is easy to use, the Lovense Lush 3 is an great option. It has an app you can download to your tablet or smartphone to operate it remotely. You can also choose the intensity and mode you want, with the added convenience of a video chat feature that lets your companion to monitor your actions.
The Lovense Lush 3 is more sturdy that its predecessor. Its sturdy, flared bottom prevents the toy from sliding through the sphincter to your penis. This toy is great for penis shaft stimulation or ball stimulation. The best way to buy a Lovense toy is to go to its official website. It is also possible to look for special offers they offer occasionally, based on where you live. You can sometimes get discounts of up to 50% on these toys.
The Lovense Lush 3 is made out of silicone, and is safe for the body. It comes with an IPX7 waterproof rating, which means it can be submerged in water for up 30 minutes. It's also easy to clean.
The Lovense Max 2 is a small device that is able to stimulate sexual activity. It comes in a barebones box, and comes with the sex toys, a USB charging cable as well as a user manual. It's not too expensive , either. The only drawback is that it's not equipped with any accessories, including cleaners or lubricants. Lovense could include these items in future models.
Max 2 Max 2 can be controlled remotely with an app called the Lovense Remote app. It lets you alter the level of vibrations and patterns for the device. It can also be synced to another device using Bluetooth. This means that you can enjoy realistic cybersex from far away. Lovense also provides a selection of other products.
The Lovense Max 2 has seven vibration modes that vary from basic to intense. You can choose which mode is most suitable for your partner. You can also alter the frequency of the vibrations in order to be more or less so.
The Lovense Gush is a portable hand-free, vibrating sextoy that provides a comfortable, all-over stimulation. Its size can be adjusted, and it has ridged edges to ensure maximum stimulation. It connects with Bluetooth to its Lovense Remote app. The app can be used to alter the Gush's patterns and manage it through your smartphone.
The Lovense Gush is designed to offer gentle vibrations that produce a pleasant buzzing sensation. It also comes with built-in music recognition to Spotify playlists. It requires 65 minutes to charge and offers 1.5 to two hours of battery life. It also requires water-based lube and pairing with Lovense. Lovense app.
Lovense Gush is easy to use and is suitable for solo play or intimate sex. It can help provide an unrestricted stimulation that allows you can focus on your partner's needs. It increases the sensations and creates larger orgasms.
Ferri Lovense is a smartphone app that allows users to communicate with others via the app. Its features include video as well as voice calls. You can send messages and vibration patterns. It can also be used to create and make voice memos. This application can be utilized by anonymous users and camera performers.
Ferri is compatible with Bluetooth 4.0 and is compatible with Mac and Windows PCs. It allows you to manage your device using an app or on your phone with your partner. The app allows you to customize the sound and pattern to create the perfect ambiance. There are four pre-programmed sound patterns to choose from. You can also adjust the speed and frequency.
The Ferri Lovense can be charged via USB or power adapter. Its charging time is of 60 minutes or about two hours, contingent on usage. The device comes with a magnetic cap and the body is sculpted. Additionally, it features a rounded edge that is designed to target pleasure points externally.
Hush can be used Hush to make your love life more exciting. It's a clever design and is easy to get rid of when finished. However, it can be quite loud especially when you turn it up to its highest setting. If you plan to utilize Hush in public, it's best to use it when you're on your own.
In order to use Hush for the first time, you'll need to sign up for an account on the application. Once you've done that, you'll be in a position to find your partner and pair your devices. From there you'll be able play with your partner's toy from a distance. You can also send your partner vibration patterns in real time. You'll have the same control as you do with Bluetooth, including loop and float features. The app lets you talk on video to your companion while you're controlling Hush.
Hush plug Hush plug is made of silicone and is water-resistant. It should be cleaned with a mild soap or sex toy cleaner. It is important to select a cleaner that is scent-free and antibacterial. Once cleaned, Hush should be dried thoroughly.
Lovense has launched a new version of their Edge Face-to-Face device. It's the Edge 2. Edge 2. Edge 2 has a number of enhancements over the previous model that include the magnetic charging port, which makes it easier to use. The new device also has an upgraded antenna design and layout for a more stable connection. The Edge is a new model that Edge features a larger bulb just above the neck, which provides more stability and P-Spot stimulation in addition to an improved battery which will last longer than the older model.
Lovense Edge 2 is operated by an app that is installed that runs on your phone. The app allows you to create vibration patterns that you can then sync to sounds or music on your phone, and wake up with an alarm that vibrates. The app can also let you control the Edge 2 from a distance. There are two apps available for controlling it, so you have the option to pick which one is the best for you.
Edge 2 Edge 2 comes with four different vibration patterns and each one has its specific intensity level. To pick the most suitable one, hold on the button to power for between three and five seconds. It will then buzz. Edge 2 will then briefly beep. The level of intensity can be adjusted by using the 4 settings for intensity and the Edge 2 has four pre-programmed patterns that you can choose from: wave, pulse fireworks, pulses, and earthquake. The app can also let users change the patterns and intensities.
It is Nora Lovense is a sexual toy that has a number of characteristics. It is constructed of medical-grade silicone that is completely safe for your body. It also comes with an ergonomic handle made of medical grade ABS plastic. The handle is ergonomic and easy to hold. And , unlike other like-minded products Nora is able to be washed using only moderate soap, water and.
Nora features a head that rotates which gently massages your g-spot while transferring the vibrations of your motor in the clitoral region. You can alter the intensity of the massage by altering the settings, including the intensity of vibration and the rotation speed. It also comes with a companion app that allows users to remotely control Nora. Using this app, you can also transfer the control to your companion through Bluetooth as well as Wifi.
Nora is equipped with a USB rechargeable battery, which can last for up to four hours of continuous use and up to 5 day of battery standby. It's made from ABS plastic and body-safe silicone , and is protected by a one-year warranty.
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Enjoy your affordable summer vacation in the beautiful Mediterranean islands of Spain.
Mallorca is the main island of the Balearic Archipelago and has great weather from spring to late autumn so you can enjoy the sun, palm trees, nightlife in one of the most popular destinations across the old continent.
Offer available in May and October for BlueAir Flights with a stopover in Torino (Tuesday, Thursday and Saturday). For a return on Saturday you can even run for a quick visit of Torino as you have a 7h 45 min stopover.


Instagram is today's premier photo-sharing app, but it has somehow lost luster amidst all the TOS changes, security, and ownership concerns. If you want to share photos that you truly own, you can host your own Instagram-like platform with Ownstagram. This photo sharing software lets you upload your pictures from the website or its own dedicated Android app, while having full ownership of your photos.
Ownstagram is a free service with high ideals. It will let you keep ownership of your own photos, free from advertisement or hidden risk. You can even download the open-source software so you can host your pics on your own. All you need is a PHP and MySQL enabled server.
Ownstagram's design language is very sleek and simple. Once you have registered with Ownstagram, you can upload photos from the website or the Android app. Once uploaded, you can share the page with a unique URL, or send the image via e-mail.
Readers viewing your images can post their own comments and view your public photos. The Android app even includes filters, just like Instagram.
Ownstagram is a timely app for anyone looking to participate in social photography without relenting to Instagram's terms of service. As more users support this format, and host clones of the project, it can slowly become a viable guilt-free alternative to Instagram.
Photo-sharing software that lets you upload from the website or Android app.
Host your own Ownstagram on your server.


Tickets for the 2016 Student Internship Program lunch, offered by Sam Houston State University, are on sale now ! Audio system this week are Mark Bentley (Risklab Australia) describing the development of quantitative danger models for cybersecurity in firms, Paul Rimba (Data61 Melbourne) on cybersecurity tech, and Marthie Grobler (Data61 Melbourne) who will talk about her work in South Africa and Australia on cybersecurity and the psychology of expertise and know-how users.
Scitech is an educational and engaging science centre conveniently located within the heart of Perth. In ExxonMobil, we believe that the key to the world's energy challenges lies in know-how and innovation. Customise your SciTech Now expertise by choosing your local PBS station under. Scitech have been a key companion in designing, commissioning and validating the ability and played a significant half in efficiently delivering a functioning facility.
SciTech Hands On Museum provides over 200 interactive science and technology exhibits. The second series of Sci+Tech in the City will be held on Thursday evenings from 4:30pm to 6:30pm, between 09 November 2017 and 30 November 2017 (inclusive). SciTech groups with small and enormous companies to be able to provide the most effective complement of capabilities for responding to the client's wants and requirements.
The Scitech Discovery Centre has remained in its present location of City West for 29 years. If you do not hear from us, please email scitech AT_TOWSON or call 410-385-6323. Her presentation's theme was Moral AI, and spoke to the significance of industry staying aware that humans are on the center of AI, and it is industry's responsibility to build ethics into the techniques and data to protect towards three threats -privateness, un-biasing, and control.


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There is no content that is not interesting
Jörgen Dahlqvist is not easy to achieve as it seems to be always moving from place to place and project to project. In addition to his role as artistic director
05 November 2019 Tuesday 01:00
Jörgen Dahlqvist is not easy to achieve as it seems to be always moving from place to place and project to project. In addition to his role as artistic director of the freedom group, Teatr Weimar and teaching at the theatre academy in Malmö, sweden, and appears to be up-to-date with the new in-house productions as playwright and director. When we all get together at the art gallery in Malmö, sweden, he'll soon be off to the united states, in order to prepare for a new generation. At the same time the approaching of even a Transistorfestival, and the eighth in the order of more than three years, with a program that, until now, has steadily expanded and evolved.
In the Transistorfestivalens the frames meet for the theater, dance, music, art, literature, and performance art. The boundaries between the arts, go to know it only when you have passed them, and says Dahlqvist.
" where The question is, what theatre really is, I've been busy right from the start. It's only when you reach the no man's land between the arts, one can clearly see this is no different than a movie theatre.
Performance = the ability to experiment,
it is also the study that is the focus of the Transistorfestivalen. This is a platform where emerging and established practitioners can try out their ideas and in unison with the others. As the initiator of the help and Jörgen Dahlqvist, in conjunction with the designer, Jan Pettersson, and producer, Anna Jonsson, sweden-Based support where it is needed. It can be of very practical assistance in the form of loans of equipment, or the advice of the artistic process.
" the Idea is that the Transistor will provide an opportunity for practitioners to experiment in peace. It is then up to them to what degree they feel they have to respond to it. Some of the work stays in the lab while others must respond to an audience.
When the Transistor goes into the fourth year, he feels that it is time to revise the direction for the future. Instead of being quick to grow and develop as in the past, he believes in a process that runs slower and slower, and to allow for in-depth studies.
" At the beginning, go on to clean and cut the pepper and the content. It is also an activity that is totally individual. Right now, several of the key jobs in the different institutions, which means that they will not be able to be involved in the work.
Teatr Weimar's veterans
free group comprises the Teatr Weimar, to the "old hands" in the region. Sixteen years have passed since they started their business in the attic of the former movie theater Panora, in the neighborhood of S:t Gertrud in Malmö, sweden.
" It was the kind of thing that went on at the time, that, at short notice, have access to a local in the heart of the city.
at Home in sweden, he had been running a record label, and based on the experiences and attitudes of the world, and he had a big advantage, when he co-founded the Teatr Weimar.
" I had been working as a graphic designer, and the capital of the business I was able to put up the first piece. I did not apply for funding but started up right away. It was the easiest thing I have ever done, is to start an order.
In quick succession, they had two plays, "A call to martyrdom," and "the Blood, the cries of their brothers ' first in the script, and the directing of his own. A long-awaited debut, if it was easy, to set up a theater, it had taken him, the longer will be the period of time to mature as a writer. And, as a director, he felt that he has a lot to learn yet.
In my early twenties, I went by accident in a training course on how to write a drama. I was obsessed with it, I could see that the actors were able to do with a piece of paper and it was felt that there was a lot of knowledge that I had, that I wanted to get to me.
During the ten-year period of time, he sent an equal number of pieces for the various players in the theatre world, were slammed, but took the criticism and tried again. It is self-reflective, constantly omprövande the approach to returns in the group's work, and he says it's a great trip, as long as the "got a feeling".
" The first years seemed to be, we are very much in the shadow of the more high-profile groups such as the Theatre of the Bulls. It gave us the opportunity to develop our character.
In Malmö, sweden, is growing near
at the same time, each kulturklimatet and once the business was up and running, the group was by today's standards, the generous funding to pursue this work further.
" today, the new groups are, perhaps, one-third of the amount of money we had in the beginning. It makes a big difference to confidence in the future.
Still, he is confident that the new artists will have to find new ways to reach out with their work. He points to the possibilities of the stream teaterupplevelser. The audiowalks, pods, and digital platforms such as the Transistor, the Sound of some of the works from the Transistorfestivalen able to survive and find a new audience, after the end of the festival. In Malmö, there is also a generosity of spirit between colleagues, he did not see the Stockholm, sweden, or Gothenburg, sweden.
" Here it is, so few people, you know that sooner or later it will have to work together. This allows the climate to become less hateful, and to a greater extent to help one another.
for Himself, he is at a stage where he was standing, and weighs from the variety of options. In recent years, he has devoted himself to teaching and collaboration with other institutions and projects. Maybe there will be more research in the future, maybe even one of the partners.
" a Lot of the things I have done in the Teatr Weimar has always been a kind of artistic research. In my role as a teacher at the theatre academy, I supervised the students. So the step is not so far away, and it could be a good way to go. I feel like for now, if that's where the urge is there. There is no desire, it is not interesting to you.
Updated Date: 05 November 2019, 01:00
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Predicting attacks before they happen
September 8, 2015 by Secure360 and UMSA
Copyright: 123rf/Paul Fleet
We've written a few articles about what steps to take after your company has been breached and how to repair damages made by attacks, but it's time to shift from defensive to offensive mode. It is natural for a company to want to work out what went wrong, acting reactively to chase the symptoms of an attack. There is a focus on the indicators of an attack and identifying the attackers, victims and damage, but this approach only addresses the problem after it has happened.
Changing the perspective
Our goal is to challenge you to predict and stop attacks before they've happened, by keeping an eye on the indicators of an attack: changes in system behavior, signs someone is probing for vulnerabilities and evidence that an attacker is acting as legitimate user. Predicting early warning signs will allow companies to contain and prevent suspicious activities before they can escalate into a full-blown attack resulting in a compromised system and data loss.
Only 24% of companies feel confident in their ability to detect an attack within minutes, and just under half said it would take days, weeks, or even months before they noticed suspicious behavior. Below we have highlighted a few common attack activities that successful organizations should be tracking in order to detect and prevent attacks before they even happen:
Internal hosts communicating with known or corrupt destinations or foreign countries where the company is not doing business.
Internal hosts communicating with external hosts using protocol or ports that are not standard.
Publically accessible or demilitarized zone hosts communicating with internal hosts, allowing data to be ex-filtrated and assets to be accessed.
Alerts that occur outside of standard business operating hours, signaling a compromised host.
Network scans by internal hosts communicating with multiple hosts in a short time frame could reveal an attacker within the network. Perimeter network defenses, such as firewalls, are rarely configured to monitor traffic on the internal network, but could be used to effectively detect the early stages of such an attack.
Multiple alarm events from a single host or duplicate events across multiple machines in the same subnet over a 24-hour period.
Repeated infections signal the presence of a rootkit or persistent compromise. If a system is cleaned and becomes re-infected within a short period of time, this could indicate an ongoing attack.
A user account that tries to log in to multiple resources in a short period of time from different regions could be a sign that the user's credentials have been compromised or that a user is causing trouble within the network.
Users trying to cover their tracks or obscure their presence within your system
Signs of ARP cache poisoning, ARP spoofing, and other man-in-the-middle attacks.
Changes in any of the following: local firewall configurations and local user accounts; listening ports, system services and drivers, startup tasks, and scheduled tasks; DNS servers or IP routings.
While the list is somewhat extensive, all of these can be early indicators of a compromised system. By focusing on the indicators of an attack, including changes in network traffic patterns or volumes or programmed access to systems used only by humans, companies can stay ahead of their attackers. With the ability to detect these indicators early on, organizations can respond to and learn from events, shifting themselves into a position of offense, rather than defense.
Filed Under: Business Continuity Management, Cybersecurity, Risk and Compliance
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Asthma is a chronic disease that affects 5.4M sufferers in the UK alone. Control of the disease can be achieved by administrating drugs (bronchodilators) using pressurised Metered Dose inhalers, often enhanced by the combined use of asthma spacer devices. These devices are mostly effective in children but their design is old, cumbersome and difficult to use, which leads to a low treatment intake with increased risk of serious complications.
Using modelling and experimental approaches, the project will investigate the link between spacer design, patient-specific respiratory system anatomy, and drug delivery. The aim is to ultimately develop a computational framework for the identification of effective and personalised devices that are easy to use, portable, discrete, attractive to the younger population, cost effective, easy to manufacture, disposable and with low environmental impact.
The project is in collaboration with ELAROS (NHS spin-off company), the Sheffield Pulmonary Vascular Disease Unit (national NHS referral centre for Clinical Pulmonary Imaging) and the Sheffield Children's Hospital.
Figure 1. CFD analysis of drug particles distribution in a typical asthma spacer (left). Comparison of CFD vs MRI data in central airways (right).
The research work will be based in the Insigneo Institute for in silico Medicine, within the Department of Mechanical Engineering. The Insigneo Institute for in silico Medicine is Europe's largest research institute dedicated entirely to the development, validation, and use of in silico medicine technologies.
The students will be working within an exciting and dynamic group of approximately 40 PhD researchers and around 8 postdoctoral research fellows undertaking a broad area of in silico medicine research with strong links to clinical centres and biomedical industry.
Applicants for the post must have (or be expected to attain) a first-class or upper second class degree in an engineering discipline. An aerospace/mechanical engineering background would be an advantage, as would experience of computational fluid dynamics, aerodynamics, or image-based computer modelling.
Please note, this position is only open to UK and EU citizens with 3 or more years residency.
This studentship covers the cost of tuition fees and provides an annual tax-free stipend at the standard UK research rate (£14,777 in 2018/19).
To apply please use our standard on-line PhD application form and indicate on your form that you are replying to this advert or email me-pgadmit@sheffield.ac.uk for further guidance on applying.
For further information about this project please contact Dr Alberto Marzo.


text:
// gulp data_structure:binary_tree:traverseWithInorder

const {
    binaryTree5,
    binaryTree6
} = require('../../mockData/binaryTree');
const { print, getPrintResult } = require('../utils.js');

/**
 * This function
 * @param {*} arr
 */

/**
 * First strategy to implement: Recursive
 *      Time complexity:
 *      Space complexity:
 *      Improvement:
 */
function traverseWithInorder(node) {
    if (!node) {
        return null;
    }

    traverseWithInorder(node.left);
    print(node.val);
    traverseWithInorder(node.right);
}

/**
 * Second strategy to implement: Iterative
 *      Time complexity:
 *      Space complexity:
 *      Improvement:
 */
function t() {}

// ========= TEST ========
const should = require('should');
traverseWithInorder(binaryTree5);
getPrintResult().should.eql([7,9,4,2,5,1,3,6,8])
traverseWithInorder(binaryTree6);
getPrintResult().should.eql([4,2,5,1,3])

module.exports = traverseWithInorder;

redpajama_set_name: RedPajamaGithub