text:
\section{Introduction}
Quantum plasmonics is a rapidly growing field studying the interaction of light with extremely small metallic systems where quantum effects come into play \cite{tame2013quantum,varas2016quantum,fitzgerald2016quantum}.
Besides investigating promising applications in chemistry \cite{hartland2017s}, photovoltaics \cite{solar_cell} or photodetection devices \cite{review_Nordlander},
an increasing amount of studies are dedicated to more fundamental topics such as the
emergence of plasmons in nano-systems \cite{varas2016quantum} or the quantization of these plasmonic excitations \cite{tame2013quantum, sundararaman2014theoretical, ballester2009long_range}.
In the simplest picture the plasmon is the optically induced collective oscillation of the
interacting electron gas against the positive background charge. In the bulk or high density limit a derivation of the plasmon on the microscopic level can be performed using density matrix theory
\cite{grosso2000solid,giuliani2008quantum,old_paper,LP_in_RPA,dasgupta1977surface,ekardt1984dynamical}. In this derivation the plasmon emerges due to Coulomb interaction between the electrons,
treated in Hartree-Fock and random phase
approximation (RPA). When the system size reaches the nanoscale the energy becomes quantized, which suggests the question: What is the impact of a discrete energy structure on the formation of
the plasmon?

To gain insight into this fundamental question, we study the dynamics of a few-electron system obtained via optical excitation of a small metal nanosphere. Experimentally, gold nanospheres can
nowadays be fabricated with sizes less than a few nm \cite{jin2015atomically,weissker2014information} and give rise to interesting nonlinear optical properties \cite{philip2012evolution,knoppe2015nonlinear, knoppe2016second}.
Current state-of-the-art techniques discussing the emergence of plasmons in nano-systems involve \textit{ab initio} methods, where the optical response of the system is calculated using time-dependent
density functional theory (TDDFT). Most of the calculations deal with few-atom systems such as one-dimensional sodium chains \cite{yan2007end, yasuike2011collectivity,bernadotte2013plasmons} or
small metal clusters \cite{ma2015interplay,Govorov_review, Gov}. To distinguish collective, plasmonic excitations from single particle electronic contributions in discrete systems is a challenge
and there are several studies trying to address the distinction between the two \cite{ma2015interplay,bursi2016quantifying,scholl2012quantum,Zhang2017}. Other studies are trying to bridge the gap between macro- and microscopic
scales by adapting classical models including electromagnetic calculations \cite{sinha2017classical} and a hydrodynamic model \cite{ciraci2016quantum,ciraci2017current} with the help of correction terms
to take into account quantum effects such as electron spill-out.

In this work, we follow a different approach to access the optical response of a few-electron system. Similar to what has been done for the bulk case, we use the density matrix formalism and include
the Coulomb interaction in Hartree-Fock approximation. In the linear regime, we study the change in
the spectral response of the system. In the non-linear regime, we
analyze the dynamics of electrons excited at the resonances, which gives rise to an oscillatory behavior strongly influenced by the Coulomb interaction. In a
diagonalized basis of the mixed states we find an oscillatory dynamics, which we compare to Rabi oscillations found in a two-level system. It turns out that the Coulomb interaction leads to strong
deviations from two-level system behavior. By explicitly treating the Coulomb terms our paper gives
valuable insight into the role of Coulomb interaction which is mostly veiled in other approaches.

The paper is organized as follows: the theoretical model is summarized in \cref{sec:theory}, introducing the model Hamiltonian, the analytical wave functions and the derivation of the density matrix
equations of motion for a nanosphere; \cref{sec:results} presents results for a nine-electron model system for two different excitation regimes. The spectral response in the linear regime is discussed
in \cref{subsec:linear}, while the dynamics in the non-linear regime is explored in \cref{subsec:nonlinear}.

\section{Theory\label{sec:theory}}

The Hamiltonian describing the system has three components
\begin{equation}
  \hat{H} = \hat{H}_{0}  + \hat{H}_{ext} + \hat{H}_{e-e}, \label{eq:H}
\end{equation}
with the single-electron Hamiltonian $\hat{H}_0$, the interaction Hamiltonian with an external field $\hat{H}_{ext}$ and the electron-electron interaction Hamiltonian $\hat{H}_{e-e}$.
The single-electron term depends on single-electron eigenenergies $\epsilon_i$ and is given by
\begin{equation}
 \hat{H}_0 = \sum_{i} \epsilon^{}_{i} \hat{c}^{\dagger}_{i} \hat{c}^{}_{i}.
\end{equation}
$\hat{c}^{\dagger}_{i}$ and $\hat{c}^{}_{i}$ are the creation and annihilation operators of an electron in a quantum state ${i}$.
We assume that the electrons are inside the sphere with radius $a$ described by a hard wall potential fulfilling the stationary Schr{\"o}dinger equation.
The solutions are given by the analytic wave functions $\psi_{i}$ with $i=(NLM)$ in spherical coordinates $\vec{r}=(r,\theta,\phi)$ with the corresponding eigenenergies
\begin{subequations}
\label{allequations}
\begin{eqnarray}
\hskip-1.5ex\psi_{NLM}(\vec{r})&=&\sqrt{\dfrac{2}{a^3}}\dfrac{1}{|j_{L+1}(x_{NL})|} j_L\left(x_{NL}\dfrac{r}{a}\right)Y_L^M(\theta,\phi)
\label{eq:wave_func} \\
   \epsilon_{NL} &=& \dfrac{\hbar^2}{2m}\left(\dfrac{x_{NL}}{a}\right)^2, \label{eq:eigenenergies}
\end{eqnarray}
\end{subequations}
where $x_{NL}$ is the $N\textrm{th}$ zero of the spherical Bessel function $j_L$ of order $L$ and $Y_{L}^M$ are the spherical harmonics. The generic set of quantum numbers $i=(NLM)$
is adopted from atomic physics and the states are classified as $s,p,d...$-shell, accordingly.
 We do not consider spin in our model. Note that the eigenenergies are $(2L+1)$-fold degenerate.

For the interaction with the external light-field, we consider an electric field polarized in z-direction and we assume dipole approximation (i.e. the field is uniformly distributed
over the volume of the nanoparticle)
\begin{equation}
 \hat{H}_{ext} = -eE(t)\sum_{ij}d^{}_{ij}\hat{c}^{\dagger}_{i}\hat{c}^{}_{j},
\end{equation}
where $d_{ij}$ is the dipole matrix element between the states $i$ and $j$. Note that we do not apply the rotating wave approximation (RWA).

The electron-electron interaction is mediated by the Coulomb potential
\begin{equation}
 \hat{H}_{e-e} = \dfrac{1}{2}\sum_{ijkl} V^{ijkl} \hat{c}^{\dagger}_{i}\hat{c}^{\dagger}_{j}\hat{c}^{}_{k}\hat{c}^{}_{l},
\end{equation}
where $V^{ijkl}$ are the Coulomb matrix elements. For the electronic states in \cref{eq:wave_func}, we can calculate
the Coulomb matrix elements by expanding the potential $\frac{1}{|\mathbf{r}-\mathbf{r'}|}$ using spherical harmonics.
For the interaction with the light field, we assume the quasi-static limit. Assuming that the light field amplitude is
in $z$-direction, the dipole selection rules apply and only states with $\Delta M=0$ and $\Delta L=\pm 1$ can be excited,
as shown in \cref{fig:en9} for the case of 20 states, i.e. states up to the $2p$-shell.

The dynamics is introduced via the Heisenberg equations of motion
\begin{equation*}
i\hbar\dfrac{d \hat{\rho}_{nm }}{dt} = [\hat{\rho}_{nm}, \hat{H}]\,,
\end{equation*}
where $\rho_{nm}=\braket{\hat{\rho}_{nm}}=\braket{\hat{c}^{\dagger}_{n}\hat{c}^{}_{m}}$ are the density matrix elements. The diagonal elements of
the density matrix represent the occupation probability of states in \cref{fig:en9}, while the off-diagonal elements represent
the coherences between them. The density matrix approach accounts for the time-dependent response of the system.

Due to its many-body nature, the Coulomb interaction leads to an infinite hierarchy of equations of motion. This is truncated on
the mean-field (Hartree-Fock) level \cite{Rossi2002}. Hence, only the single particle correlations are taken into account in the carrier-carrier interaction contribution.
Within this approximation, we obtain the following closed form of the density matrix equations of motion
\begin{align}
 i\hbar\dfrac{d \rho_{nm}}{dt} &= (\epsilon_{m}-\epsilon_n)\rho_{nm} + \nonumber\\
		  &\qquad +\sum_{i} \left( W_{m i}\rho_{n i} - W_{i n}\rho_{i m} \right) - \nonumber\\
&\qquad -eE(t)\sum_{i}\left(d_{m i}\rho_{n i}-d_{i n}\rho_{i m} \right),
\label{eq:eom_rho}
\end{align}
where $W(\rho)$ is an effective additional potential induced by the electron-electron interaction, defined as:
\begin{equation}
 W_{i j} = \sum_{k l} (V^{i k l j}-V^{k i l j})\rho_{kl}.
 \label{eq:W}
\end{equation}
The first term in \cref{eq:W} is the Hartree term, while the second one is the Fock term which accounts for the particle exchange.
Note that this equation of motion is the starting point for the derivation of the bulk plasmon, if we would take continuous states using $a\to \infty$, as found in standard textbooks \cite{grosso2000solid}.
\begin{figure}
  \includegraphics[width=\columnwidth]{figure1}
  \caption{Schematic representation of the allowed dipole transitions in a system with $9$ electrons in $20$ possible interacting states. The energy levels are drawn to scale with degenerate
  levels split artificially for clarity.\label{fig:en9}}
\end{figure}

The ground state density matrix of a non-interacting system (i.e. there is no Coulomb interaction between electrons) is diagonal. The electron-electron interaction, on the other hand,
couples the states and the interacting ground state density matrix will include these coherences.
To obtain the ground state of the interacting system, we slowly turn on the electron-electron interaction by multiplying the Coulomb term in the equations
of motion \cref{eq:eom_rho} by a switch function with values between $0$ and $1$. We use the following time-dependent switching function:
\begin{equation}
 f(t) = \dfrac{\mathrm{erf}(\alpha(t-t_0))+1}{2},
 \label{eq:switch}
\end{equation}
where the parameter $\alpha$ controls the steepness of the $\textrm{erf}$ function and $t_0$ is the time when the value of $f(t) = 1/2$.
Using a total simulation time of $2 \ \unit{ps}$ restrains $\alpha \ge 5 \ \unit{ps^{-1}}$ to assure convergence towards
the ground state. This procedure is similar to the adiabatic connection used in Kohn-Sham density functional theory, where
the non-interacting and interacting electronic systems are explicitly connected by progressively turning on the Coulomb interaction \cite{PhysRevA29, Ernzerhof1996, ad_connection_2014, PhysRevA91}.
Nevertheless, we should point out that the adiabatic connection connects eigenstates of the non-interacting and interacting systems and,
even if the system is initially in the non-interacting ground state, it may evolve towards an excited state of the interacting Hamiltonian \cite{PhysRevA29}.
However, we checked that this eigenstate is indeed the ground state by comparing it to the one obtained by minimizing the Hartree-Fock ground state energy.
Due to the level of approximation applied to the electron-electron interaction term, the two methods are equivalent.

When Coulomb interaction is included, the different states of the density matrix become mixed. We therefore apply a unitary transformation to achieve a ground state in which the density
matrix is initially diagonal. We call this the interacting basis. The tilde is related to quantities in the interacting basis hereafter, e.g. $\tilde{\rho}$ for the density matrix.
The equations of motion become
\begin{align}
 i\hbar\dfrac{d \tilde{\rho}_{nm}}{dt} &= \sum_{i} \left(\tilde{\epsilon}_{i m}\tilde{\rho}_{n i}-\tilde{\epsilon}_{n i}\tilde{\rho}_{i m}\right) + \nonumber\\
		  &\qquad +\sum_{i} \left( \tilde{W}_{m i}\tilde{\rho}_{n i} - \tilde{W}_{i n}\tilde{\rho}_{i m} \right) - \nonumber\\
&\qquad -eE(t)\sum_{i}\left(\tilde{d}_{m i}\tilde{\rho}_{n i}-\tilde{d}_{i n}\tilde{\rho}_{i m} \right),
\label{eq:eom_rho_ib}
\end{align}
where we defined a matrix $\tilde{\epsilon}$ for the single-electron term as follows
  \begin{equation}
   \tilde{\epsilon}_{ij}= \sum_{k} S^{-1}_{i k} \epsilon_{k} S_{k j}.
   \label{eq:new_eigenen}
  \end{equation}
 $S_{ij}$ are the elements of the transformation matrix. The other two terms in the equations of motion in \cref{eq:eom_rho_ib} are analogous with the ones in the non-interacting basis
 (\cref{eq:eom_rho}), with new dipole matrix elements
  \begin{equation}
   \tilde{d}_{ij} = \sum_{kl} S_{i k } d_{k l} S^{-1}_{l j}
   \label{eq:new_d}
  \end{equation}
 and new Coulomb matrix elements
  \begin{equation}
   \tilde{V}^{ijkl} = \sum_{mnop} S_{mi} S_{nj} V^{mnop} S^{-1}_{ok} S^{-1}_{pl}.
   \label{eq:new_V}
  \end{equation}

\section{Results\label{sec:results}}

\subsection{Linear response of a nine-electron system\label{subsec:linear}}
\label{subsec:lin_resp}

We consider a small sphere with radius $a=0.5 \ \unit{nm}$ and we calculate the optical response of a partially filled few-electron system.
Explicitly taking Coulomb interaction into account leads to a rather high number of indices and a complex problem. Hence, we here consider the case of 20 states,
i.e. we take into account states up to $2p$-shell (see \cref{fig:en9}). Initially, the system is filled with nine electrons up to the $1d$ subshell (spin is not considered).
The system is excited at an onset time $\mu = 0.2 \, \unit{ps}$ with a Gaussian pulse $E(t) = E_0\exp\left(-\dfrac{(t-\mu)^2}{2\tau_0^2}\right)\sin(\omega_L t)$ with
$\omega_L = 5 \times 10^{15} \, \unit{s}^{-1}$ (this is an equivalent energy  of $\hbar\omega_0 = 3.29 \, \unit{eV}$), width $\tau_0=0.25 \, \unit{fs}$ and amplitude
$E_0 = 5.00 \, \unit{mV/m}$. The intensity is sufficiently low such that we are in the linear regime. We then evaluate the optical response by calculating the total
induced macroscopic polarization $P(t)$ from the microscopic polarizations in the density matrix
\begin{equation}
 P(t) = \dfrac{e}{v}\sum_{n,m,n<m} 2 \mathscr{Re}(\rho_{nm})d_{nm}
 \label{eq:Pt}
\end{equation}
where $v=\frac{4\pi a^3}{3}$ denotes the volume of the nanosphere and $d_{nm}$ is the dipole matrix element.
Using \cref{eq:Pt}, we can calculate the linear response in the frequency domain \cite{nano-optics}
\begin{equation}
 P(\omega) =\epsilon_0 \chi(\omega) E(\omega). \label{eq:P_omega}
\end{equation}

The linear spectrum for the two cases, non-interacting, i.e. when there is no Coulomb interaction, and interacting, i.e. when Coulomb interaction is present between electrons,
is shown in \cref{fig:lin_resp}(a). The values displayed on the y-axis are on a logarithmic scale. In the non-interacting case, the spectrum (black curve) contains transitions
between an empty and a filled state. These occur at the frequencies $\omega_{1d,1f}$, $\omega_{1p,2s}$, $\omega_{1d,2p}$ and $\omega_{1s,2p}$, as also indicated in \cref{fig:en9}.
The spectrum in \cref{fig:lin_resp} shows discrete resonances at exactly the aforementioned frequencies. The resonances have been labeled and added with dashed lines to \cref{fig:lin_resp}(a).
The strength of the peaks corresponds to the magnitude of the dipole matrix element $d_{nm}$ and the main peak is the transition between the highest occupied level and
lowest unoccupied one, i.e. $\omega_{1d,1f}$. This is a transition involving multiple states, where the five-fold degenerate $1d$ shell interacts with five out of the
seven states of $1f$ with $m=\pm2,\pm1 \, \textrm{and} \, 0$, according to the dipole selection rules. Thus, the first resonance is composed of the transitions
$7 \rightarrow 14$ (corresponding to $\omega_{1d}^{m=0} \rightarrow \omega_{1f}^{m=0}$), $6 \rightarrow 13$ and $8 \rightarrow 15$ ($\omega_{1d}^{m=\pm1}\rightarrow \omega_{1f}^{m=\pm1}$),
$5 \rightarrow 12$ and $9 \rightarrow 16$ ($\omega_{1d}^{m=\pm 2}\rightarrow \omega_{1f}^{m=\pm 2}$, respectively). Similarly for the third resonance, which involves three states.
For simplicity, we will only discuss the states with $m=0$ in our further analysis, but the behavior is consistent for all degenerate states.

When the electron-electron interaction is included, the spectrum is blue-shifted (\cref{fig:lin_resp}(a), green curve). Again we find three resonances at $\omega_{1st} = 4.84\times 10^{15} \,
\unit{s}^{-1}$, $\omega_{2nd} = 12.06 \times 10^{15} \, \unit{s}^{-1}$, $\omega_{3rd} = 15.63 \times 10^{15} \, \unit{s}^{-1}$ and $\omega_{4th} = 20.46 \times 10^{15} \, \unit{s}^{-1}$.
The discrete resonances cannot be associated with transitions
between eigenstates of the interacting multi-level system, unlike in the non-interacting case. This is shown by looking at the coherences induced between states by the external light-field in
the frequency domain. As an example, \cref{fig:lin_resp}(b) shows the spectrum of the polarization $\rho_{7,14}(\omega)$. For the non-interacting case it corresponds, as expected, to the peak at
lowest energy, confirming that here we, indeed, see the transition between those two states. For the interacting case, we find four peaks at the shifted energies. Now, two effects come into play:
first, the Coulomb interaction renormalizes the transition energies between the states leading to a shift, and second and even more interesting, it mixes the response of the individual states,
indicating the formation of a collective oscillation. Therefore, we conclude that, in the interacting system, the components of the response spectrum cannot be individually assigned to any induced
coherence. Each coherence contributes to the whole spectrum. This is observed for the other three coherences as well, as shown in \cref{fig:lin_resp} (c), (d) and (e).
We stress out that also in the interacting basis all four coherences ($\tilde{\rho}_{7,14}$, $\tilde{\rho}_{3,10}$, $\tilde{\rho}_{7,19}$ and $\tilde{\rho}_{1,19}$) contribute to each peak.
 \begin{figure}
  \includegraphics[width=\columnwidth]{figure2}
  \caption{(a) Total induced dielectric susceptibility $\chi(\omega)$ as a function of frequency $\omega$ and energy $\epsilon$ in a system with 9 electrons in 20 states
  with (green) and without (black) Coulomb interaction.(b,c,d, e) The Fourier transform of the light-induced coherences (b) $\rho_{7,14}$ , (c) $\rho_{3,10}$, (d) $\rho_{7,19}$
  and (e) $\rho_{1,19}$ with (blue) and without (dotted red) Coulomb interaction. The values on the y-axis are on logarithmic scale.\label{fig:lin_resp}}
\end{figure}

In order to further investigate the influence of the Coulomb interaction, we introduce a scaling factor $f \in \left[ 0,1 \right]$ multiplied to the Coulomb coupling strength,
i.e. for $f=0$ we are in the non-interacting case and for $f=1$ in the fully interacting case. Figure \ref{fig:Coulomb_scaling}(a) shows the spectrum for different $f$.
We can see that the four peaks blue-shift for increasing $f$, i.e., for increasing Coulomb interaction strength. The shift is smooth and derives from the non-interacting peaks.
The peak position as function of scaling factor $f$ is extracted in Fig.~\ref{fig:Coulomb_scaling}(b) (solid lines). We make two observations: for each of the four peaks the shift
occurs with a different slope and the shift is not strictly linear.

For a better understanding, we compare these findings to the eigenvalues ${\cal E}$ of the interacting Hamiltonian $H_I = H_0 + W(\rho^{(0)})$ with $\rho^{(0)}$ being the density
matrix of the Coulomb correlated ground state. Note that the eigenvalues ${\cal{E}}$ cannot be directly compared to the matrix elements of $\tilde{\epsilon}$ obtained by diagonalizing
the interacting initial state defined in \cref{sec:theory}. If the Coulomb interaction only leads to energy renormalization we would expect that the peak positions of the spectrum agree
with the energy difference of the eigenvalues $\hbar\omega^{\cal{E}}_{ij}={\cal{E}}_{j}-{\cal{E}}_{i}$. Seeing that the Coulomb correlated state can be traced back to the non-interacting
states, we consider the states corresponding to the dipole transitions $\omega^{\cal{E}}_{7,14}$, $\omega^{\cal{E}}_{3,10}$, $\omega^{\cal{E}}_{7,19}$ and $\omega^{\cal{E}}_{1,19}$.

The comparison between the peak position (solid lines) and the eigenvalue difference (dashed lines) is shown in Fig.~\ref{fig:Coulomb_scaling}(b).
Naturally for the non-interacting case of $f=0$ the two curves agree.
But for $f\neq 0$ we find a strong disagreement between the two curves, where the peak positions are always below the eigenvalue difference.
A noticeable feature occurs for a scaling factor $f\approx 0.3$, where the second and third peaks in the polarization spectrum show an anti-crossing in \cref{fig:Coulomb_scaling}(a).
This is due to the fact that the Coulomb interaction changes the order of the $2s$ and $1f$ orbitals as it can be verified by checking the order of the eigenvalues ${\cal E}$ of the interacting Hamiltonian $H_I$.
Indeed, around $f=0.3$, the blue dashed curve $\omega^{\cal{E}}_{3,10}$ in \cref{fig:Coulomb_scaling}(b) bents, indicating where the swap occurs.
 \begin{figure}
  \includegraphics[width=\columnwidth]{figure3}
  \caption{(a) Shifting of the total induced macroscopic polarization $P(\omega)$ as a function of the scaling factor $f$ of the Coulomb interaction in a system with 9 electrons in 20 states.
  (b) Comparison of the peak positions in the optical response (solid lines) and the eigenvalue difference of the interacting Hamiltonian (dashed lines) as a function of the scaling factor $f$ of
  the Coulomb interaction. \label{fig:Coulomb_scaling}}
\end{figure}
This mismatch between the eigenenergies and the polarization spectra is reminiscent of excitons in semiconductors whose spectral response always lies below the band gap.
Excitons are a many-particle phenomena, where the Coulomb interaction correlates the
individual electron energies to form a collective, bound state. This indicates the importance of the non-linear effects induced by the Coulomb interaction as well as the state mixing. It is also
a hint for collectivity in the system, because all states contribute to the formation of the peaks.

\subsection{Non-linear response of a nine-electron system\label{subsec:nonlinear}}

In this section, we analyze the optical response of the system beyond the linear regime. We calculate the density matrix time-evolution for a strong excitation at each of the four resonances in the
interacting polarization spectrum (\cref{fig:lin_resp}a)) under a continuous wave excitation that is switched on instantaneously. Accordingly we are interested in the response to excitations at
$\omega_{1st} = 4.84 \times 10^{15} \ \unit{s}^{-1}$, $\omega_{2nd} = 12.06 \times 10^{15} \ \unit{s}^{-1}$, $\omega_{3rd} = 15.63 \times 10^{15} \ \unit{s}^{-1}$ and $\omega_{4th} = 20.46
\times 10^{15} \, \unit{s}^{-1}$. The corresponding electric field reads $E(t) = E_0\sin(\omega_L t)\Theta(t)$ with $E_0$ being the amplitude, $\omega_L$ the frequency of the field and
$\Theta(t)$ the Heaviside function.

\begin{figure}[t]
  \includegraphics[width=\columnwidth]{figure4}
  \caption{Population dynamics in (a) the non-interacting and (b) the interacting basis excited by a pulse with amplitude $E_0=10^9 \ \unit{V/m}$ and frequency
  $\omega_L=\omega_{1st}$ with (c) the corresponding electric field.\label{fig:pop_dyn}}
\end{figure}

We start by analyzing an excitation with frequency close to the first peak in the absorption spectrum $\omega_{1st}$. In the non-interacting basis due to the adiabatic switch-on into the Coulomb
correlated basis, not only the lowest nine states are occupied, but most states have a finite initial occupation. When the electric field sets in, an oscillatory dynamics is initiated, as can be
seen in \cref{fig:pop_dyn}(a), induced by a light field with a frequency at $\omega_L=\omega_{1st}$ and an amplitude $E_0=10^9 \ \unit{V/m}$ displayed in \cref{fig:pop_dyn}(c).
The strongest oscillation occurs between the states in $1d$ and $1f$ and, similarly with the non-interacting case, it is the main contributor to the first peak in the linear response spectrum.
The superimposed fast oscillation can be traced back to the fact that we do not perform the RWA. Additionally all the other states start to oscillate showing that they contribute
to the dynamics in a non-trivial way. In the non-interacting basis, we can still attribute the oscillation of all states to the state mixing in the initial state.
This is in agreement with our finding in the linear regime, where we also found that several states contribute to a single peak.

Now we switch to the interacting basis, where the initial state is diagonal. This allows us to study the question, whether we can describe the system by an excitation between only two Coulomb-correlated states.
Figure~\ref{fig:pop_dyn}(b) shows the population dynamics of the density matrix in the interacting basis $\tilde{\rho}(t)$. We find that the population exchange occurs mainly between the $1d$ and $1f$
interacting states, $\tilde{\rho}_{1d}^{m=\pm2,\pm1,0}$ and $\tilde{\rho}_{1f}^{m=\pm2,\pm1,0}$ (red and blue curves in \cref{fig:pop_dyn}(b)), again because $\tilde{\rho}_{1d,1f}$ is the strongest dipole-allowed
transition in the system.
We also observe oscillations with a much lower amplitude of other states like $\tilde{\rho}_{1p}$, $\tilde{\rho}_{1s}$ and $\tilde{\rho}_{2p}$, which also have a dipole matrix element between them.

An oscillation amplitude of $\approx 1$ between the states $\tilde{\rho}_{7,7}$ and $\tilde{\rho}_{14,14}$ can be achieved by slightly changing the excitation frequency to $\omega_L=5.07\times 10^{15}
\, \unit{s}^{-1}> \omega_{1st}$, which is slightly higher than the resonance frequency found in the linear regime.
Nevertheless, even for this excitation condition, there is no perfect inversion of the system between $0$ and $1$ for the occupation of $\tilde{\rho}_{14,14}$. This is because of the many-body character of
the electronic system where the population transfer occurs between multiple states, mediated by either a dipole or a Coulomb matrix element.
The occupation approximately follows a pure sine (or cosine) behavior. We confirm these findings by a Fourier analysis of the oscillation. We consider the Fourier
expansion $\tilde{\rho}(t) = a_0+\sum_n a_n\cos\left(n\Omega_0 t\right)$ of the oscillation. Only $a_0=0.5$ and $a_1=0.5$ are different from $0$, resulting in the Fourier function
$ = 0.5+ 0.5 \cos\left(n\Omega_0 t\right)$ with $\Omega_0=1.26\times 10^{14} \, \unit{s^{-1}}$. This is displayed in Fig.~\ref{fig:F_comp1}, where we show the Fourier expansion up to order $n=4$ and compare it to a
single oscillation of the dynamics.
In order to get rid of the small oscillations which are present because we have not performed the RWA and because of the degeneracy of the states involved in the interaction,
we extract the envelope of one of the cycles of the time dynamics.

 \begin{figure}[t]
  \includegraphics[width=\columnwidth]{figure5}
  \caption{a) Single oscillation of the occupations $\tilde{\rho}_{7,7}$ and $\tilde{\rho}_{14,14}$ for an excitation frequency $\omega_L = 5.07 \times 10^{15} \ \unit{s}^{-1}$ and
  $E_0=3.4\times 10^{8}\ \unit{V/m}$ ($\Omega^{7,14}/\omega_{1st} = 0.0178$).
  b) Comparison with the Fourier expansion of the occupation $\tilde{\rho}_{14,14}$ up to order $n$ with the cosine coefficients $a_n$ as inset.
  \label{fig:F_comp1}}
\end{figure}

To analyze the oscillations in a more systematic way, we sweep the excitation frequency of the light field through the resonance. From the time-series of $\tilde{\rho}_{14,14}$ (note that $\tilde{\rho}_{7,7}$
behaves analogous, as well as all the other states in $1d$ and $1f$) we extract the frequency $\Omega^{7,14}=\dfrac{2\pi}{\tau^{7,14}}$ with $\tau^{7,14}$ being the period as well as the amplitude
$\Lambda^{7,14}=\textrm{max}(\tilde{\rho}_{14,14})$ of the oscillation for two different excitation strengths $\Omega^{7,14}/\omega_{1st} = 0.0035$ (corresponding to a light-field amplitude
$E_0=6.8 \times 10^7 \, \unit{V/m}$) shown in Fig.~\ref{fig:RO_1st_peak} (left column) and
$\Omega^{7,14}/\omega_{1st} = 0.0178$ ($E_0=3.4 \times 10^8 \, \unit{V/m}$) shown in Fig.~\ref{fig:RO_1st_peak} (right column). The ratio between the Rabi frequency and the light frequency gives
a relative measure of how excited the system is at a certain light frequency and intensity, beyond the absolute value of the field strength and the dipole moment of the transition. In this way,
we can compare different resonances in the light-induced polarization at approximately the same excitation conditions.
For the stronger excitation regime (right column in Fig.~\ref{fig:RO_1st_peak}) we see a resonant behavior with a minimal frequency $\Omega^{7,14}$ and an amplitude of $\Lambda^{7,14}=0.9$
occurring at $\omega_{1st}=5.07 \times 10^{15}$, which is slightly higher than the resonance frequency found in the linear regime. Similarly for the weaker excitation (left column in Fig.~\ref{fig:RO_1st_peak}),
where the resonance shifts to $\omega_{1st}=4.94 \times 10^{15}$. Nevertheless, the state is only partially occupied $\Lambda^{7,14}=0.25$.

The oscillations in \cref{fig:pop_dyn}b) indicate that the population dynamics of the interacting states behaves similarly to a two-level system (TLS) showing Rabi oscillations.
For a resonant excitation, the Rabi frequency in a TLS is defined as $\Omega_0 = e|\tilde{d}_{i j}|E_0/\hbar$ with $\tilde{d}_{ij}$ the dipole matrix element in the interacting basis (cf. \cref{eq:new_d}).
The generalized Rabi frequency is then
\begin{equation}
 \Omega^{TLS} = \sqrt{(\Omega_0^{TLS})^2 + \Delta^2},
 \label{eq:Rabi_TLS}
\end{equation}
where $\Delta = \omega - \omega_0$ is the detuning from the resonant frequency $\omega_0$. Remember, that only for $\Delta=0$ the oscillation amplitude in a TLS is $\Lambda^{TLS}=1$.
For off-resonant excitation the amplitude $\Lambda^{TLS}$ is given by
\begin{equation}
 \Lambda^{TLS} = \dfrac{\Omega_0^2}{\Omega_0^2+\Delta^2}\,.
 \label{eq:Rabi_amplitude}
\end{equation}

We now compare our findings of the frequency sweep to the Rabi oscillations in a TLS. For the TLS we take the peak position at $\omega_0=\omega_{1st}= 4.84 \times 10^{15} \, \unit{s}^{-1}$
as resonance frequency. We start with the right column in Fig.~\ref{fig:RO_1st_peak}. For this large excitation strength the oscillations of the occupations become faster.
This leads to an effective higher occupation of the previously unoccupied states
and in return modifies the Coulomb interaction resulting in a shifted curve and the observed differences. As opposed to a simple two-level system, there is an unstable excitation window where the occupation
is large and the Rabi frequency is fluctuating, followed by a discontinuous drop in amplitude (increase in frequency).
Thus, the Coulomb interaction influences the dynamics of the system in a complex way.

The weaker excitation $\Omega^{7,14}/\omega_{1st} = 0.0035$ (see \cref{fig:RO_1st_peak}a) and c)) behaves less pronounced. For a large range of values of excitation frequency $\omega$ away from resonance
we find an excellent agreement between the extracted values and the prediction via the TLS. However, close to resonance these two pictures deviate strongly. The minimal oscillation frequency $\Omega$
and the maximal amplitude $\Lambda$ is again shifted to higher excitation frequencies compared to the predictions of the TLS $\Omega^{TLS}$ and $\Lambda^{TLS}$.
Remarkably, the amplitude always stays far below 1 with the highest $\Lambda^{7,14}=0.25$.
We attribute this to the change in occupations
leading to a change in the Coulomb interaction which dynamically shifts the resonance frequency. Note also that the slope of the two curves are different: while the TLS exhibits a symmetric behavior
with respect to the resonance, the extracted values show a kink. This again hints towards non-linear and collective effects induced by the Coulomb interaction that is not simply a shift in resonance frequency.

\begin{figure}[t]
 \includegraphics[width=\columnwidth]{figure6}
  \caption{a), b) Frequency $\Omega$ and c), d) amplitude $\Lambda$ for excitations close to the first peak $\omega_{1st}$ for an excitation with $\Omega^{7,14}/\omega_{1st} = 0.0035$ (left, blue curves)
  and $\Omega^{7,14}/\omega_{1st} = 0.0178$ (right, red curves). The solid lines are the extracted values from the dynamics $\Omega^{7,14}$ and $\Lambda^{7,14}$ and the dotted lines are from the TLS
  $\Omega^{TLS}$ and $\Lambda^{TLS}$.\label{fig:RO_1st_peak}}
\end{figure}

\begin{figure}[t]
\includegraphics[width=\columnwidth]{figure7}
  \caption{Same as \cref{fig:RO_1st_peak}, but for excitations close to the third peaks $\omega_{3rd}$. We consider  $\Omega^{3,10}$ and $\Lambda^{3,10}$.  \label{fig:RO_3rd_peak}}
\end{figure}

Next, we want to consider what happens if we excite the system with frequencies close to the third peak at $\omega_{3rd}=15.63\times 10^{15} \ \unit{s}^{-1}$. We remark that the findings are similar to what
happens at the second and fourth peak which we therefore do not show. Again, we find an oscillatory behavior in the occupation of the states, this time the main oscillation in the
interacting basis happens between $\tilde{\rho}_{3,3}$ and $\tilde{\rho}_{10,10}$ in agreement with the dipole moment $\tilde{d}_{1p,2s}$ corresponding to this transition. Although
this transition contributes to the second peak in the $\chi(\omega)$ spectrum in the case without Coulomb interaction, it becomes the main contributor to the third peak in the case
with Coulomb interaction. This is due to the change in the order of the $2s$ and $1f$ orbitals, as explained at the end of \cref{subsec:lin_resp}.

Therefore we do a systematic analysis of the frequency $\Omega^{3,10}$ and amplitude $\Lambda^{3,10}$ corresponding to the dynamics of the population of $\tilde{\rho}_{10,10}$.
The corresponding results are shown in Fig.~\ref{fig:RO_3rd_peak} for two different pulse strengths such that the ratios $\Omega^{3,10}/\omega_{3rd}$ are the same as for the first peak.
We again compare our findings to the behavior of a TLS, here taken with a resonance frequency of $\omega_0=\omega_{3rd}$.

In Fig.~\ref{fig:RO_3rd_peak} (right column) we consider an excitation with a light field $E_0 = 5 \times 10^9 \, \unit{V/m}$ inducing a ratio $\Omega^{3,10}/\omega_{3rd}=0.0178$.
Again, there is a strong discrepancy between our system and the theoretical two-level system. There is almost total population inversion for an extended excitation window, with an asymmetric
and discontinuous excursion amplitude. This time, the kink is towards lower frequencies.

For the weaker regime, $\Omega^{3,10}/\omega_{3rd}=0.0035$ and the corresponding absolute field strength $E_0 = 10^9 \, \unit{V/m}$, far off the resonance the extracted values and the TLS prediction agree well,
while close to the resonance we see a kink in the frequency behavior of $\Omega^{3,10}$. The amplitude always stays far below 1 with the highest $\Lambda^{3,10}=0.45$.

\begin{figure}[t]
  \includegraphics[width=\columnwidth]{figure8}
  \caption{a) Population dynamics of $\tilde{\rho}_{3,3}$ and $\tilde{\rho}_{10,10}$ for an excitation at $\omega_L = 15.45 \times 10^{15} \ \unit{s}^{-1}$
  and  $E_0 = 10^9 \, \unit{V/m}$ ($\Omega^{3,10}/\omega_{3rd}=0.0035$).
  b) Fourier series $\tilde{\rho}_{10,10}$, where each curve $a_n$ implies that cosine coefficients up to order $n$ have been added to the Fourier series with the values of the cosine coefficients $a_n$ as inset.
 \label{fig:F_comp3}}
\end{figure}

Finally, let us have a closer look at the population dynamics of the contributing states $\tilde{\rho}_{3,3}$ and $\tilde{\rho}_{10,10}$ in the interacting basis.
Two periods of the oscillation are shown in \cref{fig:F_comp3} induced by a field at the maximal amplitude using $\omega_L = 15.45 \times 10^{15} \ \unit{s}^{-1}$
and $\Omega^{3,10}/\omega_{3rd}=0.0035$. The dynamics is similar for $\tilde{\rho}_{7,7}$ and $\tilde{\rho}_{14,14}$ at maximum amplitude and same excitation regime.
Already here, we clearly see that the dynamical behavior deviates in
an interesting way from the sine-behavior found in a TLS. It is more bell-shaped.
Similar bell-shaped oscillations have been found in the Rabi oscillations in semiconductor quantum dots under local fields,
which likewise result from the non-linear term in the Bloch equations \cite{Slepyan2004}. When we do a Fourier analysis of
this curve, we find that higher harmonics contribute strongly to the formation of the dynamics, in this case up to sixth
order. This can again be traced back to the Coulomb interaction, which has more influence when the pulse strength is weaker.
Hence, the influence of the Coulomb interaction leads to non-linear effects like the instantaneous formation of higher
harmonics for the light-induced changes in the occupation.
Although pumping the system harder reduces the order of the Rabi frequency harmonics induced (cf. \cref{fig:F_comp1}),
the non-linear effects are still manifesting via the asymmetric occupations as a function of the excitation frequency and the
complex time-dynamics around the resonance.

We emphasize that we distinguish two types of non-linear effects in our system: higher harmonics of the Rabi oscillations' frequency and dynamical shift
of the resonance frequency. The two effects are competing with each other since both the Coulomb interaction and the light-field are driving the dynamics via the Hamiltonian.
Hence, for weaker excitation, the Coulomb interaction dominates, resulting in the bell-shaped dynamics, while a stronger one
drives the oscillations closer to an optical two-level system excitation.

To conclude this section, we comment on our method in relation to DFT methods. We remark that our formulation takes into account a bare Coulomb potential calculated
explicitly from the analytical single-electron states within the Hartree-Fock (exchange) approximation. In contrast, in DFT going
beyond Hartree approximation involves considering an exchange-correlation
 functional such as the local density approximation (LDA). Within this approximation, a DFT ground state is calculated, from which a linear response can be obtained.
 Because the ground state from our method and the DFT ground state can differ quite significantly, we expect also quite different
results comparing the two methods. To calculate the dynamics, it is possible to use (real-time) time-dependent (RT-TDDFT) codes.
In these calculations, the exchange-correlation functional is again a crucial ingredient, which due to its dynamical shift has to be treated with great care \cite{
ruggenthaler2009rabi,fuks2011nonlinear,provorse2016electron}, while our approach is well suited to study dynamics. We would also like to remark that in DFT
studies the coherences between the states might be lost due to the reduction to the electronic density, while in our dynamics we naturally keep
all the coherences between the states.

While the TDDFT methods are widely used in the study of quantum plasmonic systems, the density matrix approach is a well-established method in the field
 of optically excited semiconductors, particularly to describe Coulomb effects like excitons and band gap renormalization \cite{Rossi2002,haug2009quantum}. Due
 to the discrete energy levels in our system and the finite gap between the highest occupied and lowest unoccupied state, the system is somewhere in between a
 metal and a semiconductor.

\section{Conclusions}

In summary, we have used a microscopic density matrix formalism to describe the electrons dynamics in a quantized nanoparticle. The methodology is similar
to the one used for the derivation of bulk plasmons. We considered a system of $9$ electrons with an explicit description of the Coulomb
interaction on the mean field level and studied the effects of the Coulomb interaction on the optically induced dynamics. In the linear regime,
the Coulomb interaction leads to a shift of the resonances and a state mixing, indicating a collective response. In the non-linear regime, the optically
induced oscillations of the occupation were strongly modified due to the Coulomb interaction.

Our study lies in between two limiting cases: in one limit, one considers one or two electrons which then results in the description of Rabi oscillations
and a formulation using a two-level system. Such a description is used successfully, for example, to describe semiconductor quantum dots. In the other limit,
one considers many-electron systems where plasmons are described within the RPA, and a classical treatment of the material polarizability is usually sufficient.
Neither of the aforementioned descriptions is sufficient to describe the Coulomb effects in a few-electron system, underlined by the fact that our findings
deviate from both limiting cases. Instead, we find similarities with both cases. For certain excitation conditions the system behaves like the two-level
system exhibiting Rabi-oscillations. On the other hand, we find hints for collective behavior, like energy shifts and the modification of the oscillations,
which are typical for plasmons.

\section*{Acknowledgments}
This work was supported by the EPSRC through EP/L027151/1.
We are grateful to Benjamin Burnett and Stefano Guazzotti for most fruitful discussions. A. Crai thanks Johannes Lischner for the helpful advice.
D.E.R. is grateful for financial support from the German Academic Exchange Service (DAAD) within the P.R.I.M.E. programme.

redpajama_set_name: RedPajamaArXiv


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Russia launches fresh diplomatic counter-offensive to win back influence lost after the Arab Spring.
The first Russian-Arab Cooperation Forum took place in Moscow on Feb. 20. In attempts to regain the position in the region that it lost after the Arab Spring, Russia has been trying to revive both the Palestinian-Israeli and the Syrian regime-opposition dialogues. Experts are skeptical, believing Moscow's activities will only help improve its image.
Moscow waited three years for a meeting with Arab world representatives on Russian soil. As he opened the first session of the Russian-Arab Cooperation Forum at the ministerial level, Russian Foreign Minister Sergei Lavrov reminded the audience about the region's key problems.
Lavrov said that Moscow's initiatives regarding those problems have, until now, been either rejected by the Arab world (as happened in the Syrian crisis) or hampered by Israeli obstruction (as in the Palestinian-Israeli process and the idea of a nuclear-free zone conference).
In his address to the Arab ministers led by Arab League Secretary General Nabil Elaraby, Lavrov made it clear that Moscow would not remain on the defensive: instead of fighting accusations of collaboration with the Assad regime, it is beginning a diplomatic counter-offensive.
The situation in Syria — where the fighting between President Assad and the opposition has deadlocked — has justified grounds for this. In Moscow's opinion, this makes the Russian idea of an internal Syrian settlement (as an alternative to a violent ouster of the Syrian regime with the help of outside forces) increasingly viable.
"It's possible to conclude that betting on a resolution by force from either side isn't working. An understanding that dialogue must begin is increasingly gaining ground," Lavrov said of the new trend.
The Syrian crisis was a subject of a recent telephone conversation between Lavrov and U.S. Secretary of State John Kerry.
Having diverged radically on Syria over the past six months, Moscow and Washington must now look for points of convergence. For now, their positions are still far apart. According to the Department of State spokesperson, Victoria Nuland, the Secretary of State (who will start a tour of Europe and the Middle East on Feb. 24) will take part in a meeting with the leaders of the Syrian opposition in Rome.
On the eve of the Russian-Arab Forum, Sergei Lavrov announced the visit of the Syrian minister to Moscow, which is expected on Feb. 25. He added that the Russian side intended to discuss issues to be resolved, in order to start a dialogue in Syria.
"We are working in this direction with the opposition too, and we have never stopped working with the government and with those who oppose it," Russia's foreign minister said.
However, experts are skeptical concerning Moscow's renewed activity in the Middle East.
"The existence of a few dozen Arab countries in the world is very useful for Russia's Foreign Ministry. First of all, this allows it to keep an army of Arabic-specialist diplomats on the payroll. Second of all, this gives Moscow an opportunity to be present among the strong nations of the world as a co-sponsor of the Middle East peace process, which is an honor — yet quite meaningless for the Palestinian-Israeli settlement as such," said Evgeny Satanovsky, president of the Middle East Institute.
"At the same time, none of this rules out the participants manoeuvring around Russia, which is exactly what we see today," said Satanovsky.
The article is first published in Russian in Kommersant.


text:
Margarito Tereré es una película de Argentina filmada en Eastmancolor dirigida por Waldo Belloso según su propio guion escrito en colaboración con Zulema Alcayaga que se estrenó el 27 de julio de 1978 y que tuvo como actores principales a Jovita Díaz y Armando Guerisoli.

Sinopsis
La abuela del yacaré Margarito le deja como herencia un cofre cerrado y una carta.

Reparto

Comentarios
ML en La Prensa escribió:
La Razón opinó:
Manrupe y Portela escriben:

Referencias

Enlaces externos
 Información sobre Margarito Tereré en el sitio del cine nacional
 Información sobre Margarito Tereré en Internet Movie Data Base

Películas infantiles

redpajama_set_name: RedPajamaWikipedia


text:
Herbert T's
72 Years Active Service
96 years wasn't quite enough time for Herbert Tanner to perfect his barbecue sauce. It was enough time to serve 72 years as a Volunteer Fire Chief and Methodist deacon, and dang sure long enough to become a great-grandfather. But tinkering with his vinegar-based sauce, developed over years in his kitchen in Hemingway, SC, was something he could just never stop doing.
Luckily his grandson, Ben Tanner, was paying attention to all of Herbert's recipe variations.
When he first started making his own sauce, Ben took the best bits and pieces of each of Herbert's ingredients and made it into something palatable.
The roots of open-fire barbecue are in the lowcountry of South Carolina, and while it might have been a 16th Century joint venture between the Spanish and Native Americans that produced the first known vinegar-based barbecue sauce, it's been refined and mass produced for hundreds of years now.
It's only recently been perfected with Herbert T's. It's the sauce that takes you back to Herbert's kitchen and the search for something ideal. Back to Ben's efforts to keep that legacy living. Back to the very roots of barbecue flavoring.
It's about time.
Mr. W. Herbert Tanner
W. Herbert Tanner is the inspiration of our "little bit of heat". He worked 72 years with the Hemingway volunteer fire department. Mr. Herbert managed to answer calls every time he came home on military leave and was considered a permanent member of the department because his chief knew one day soon Herbert would come home for good to serve out his life as a fireman. Eventually he became chief of the department. Mr. Herbert was known for the mark he left on the department forever. One story that remains a favorite is the tale of Mr. Herbert feuding with the police chief. It seems that Mr. Herbert always parked his pickup truck conspicuously in front of the fire station in a location that was marked in a yellow no parking area. The police chief frequently picked at Mr. Herbert for his disregard of the law, and on one occasion even wrote the chief a parking ticket. Not to be outdone, Mr. Herbert placed a sign affixed to the side of the fire station which settled the dispute once and for all. "Don't even think of parking here" still remains on the side of the department building to this day. Chief W. Herbert Tanner passed away at the age of 96 and his memory continues to live on for many.
We hope to preserve the legacy Mr. Herbert left behind and we'll think of him every time we open up another bottle of Herbert T's.
In the press: The Beaufort Gazette, April 2018
sauceboss@herbertts.com

redpajama_set_name: RedPajamaCommonCrawl


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Model G-2 - Version without the large storage drawer.


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text:
Full Tilt Manager Shares Details On Reward Program
12 October 2012 by CasinoListings
Online poker site Full Tilt Poker's Manager took part in an online forum to give players some details on the site's new Full Tilt Reward Program which is set to launch with the new site in November.
Shyam Markus shared that the reward program is not something that came from the purchasing of the company by PokerStars, but was instead something that Full Tilt had been working on before it was crippled by US authorities on Black Friday.
The program will include weekly cash payments which are based on the amount of Full Tilt Points that players earn throughout each week. $2.50 is set to be awarded for every 100 Full Tilt Points awarded.
More details revealed by Markus about the program included:
"Unlike affiliate-paid rakeback, there are no deductions of fees (store purchases, promotions, etc, therefore, the 25% mentioned above will almost always beat the 27% that rakeback was giving, he said.
Because the weekly cash payments are now based on points earned, FTP's will now be earned using the Weighted Contributed method instead of the Dealt method.
The weekly cash payments don't use up the FTP's earned, so players can still spend them in the store. Depending on how they are spent, points add an additional 4-5% to the program, giving the top level of the new program a giveback of up to 30%.
Since there are no fee deductions, all FTP's are worth more to former rakeback players than previously, which increases the value of promotions like Happy Hour and Take 2.
Full Tilt will have a transition from Iron Man and Black Card to this new program, so long-term players of both promotions will likely get a leg up in the new program from the start.
The top level of this program is significantly easier to achieve than Black Card was. The Black Card store will be changed so that anyone in the new top level can use it. This means that more players will be eligible to purchase cash bonuses in the store.
If player's qualified for the 2011 Iron Man Mid-Year Bonus, they will still receive it when the site re-launches.
The Black Card program will return (not at re-launch, but eventually) in a brand new way. Expect a little news about that soon."
The manager also went on to answer player questions about the upcoming re-launch of Full Tilt, and revealed that:
Players will be able to download, install and even log in before November 6th, to be sure the system runs smoothly at launch
Log-in PIN will still be in effect
FTP Lobby will not have changed
Multi currency cashier is in the pipeline
A fulltiltpoker.eu website is one of the company's highest priorities and can be expected in one of the early updates following re-launch
Pairing Full Tilt and PokerStars accounts will involve logging in to both sites and using a pairing code to link the accounts, but more information will be released when this is available.


text:
Here are the first photographs of Prince Harry after his honeymoon with Meghan Markle
He was photographed at charity gala in London
Prince Harry and Meghan Markle have reportedly just returned from their honeymoon and are already back to business. Particularly, the new Duke of Sussex has immediately jumped back into his philanthropic pursuits.
Harry attended a charity gala in London Thursday, and several attendees at the event shared some of the photographs they snuck of the Prince on social media.
"Encouraging #onsideyouthzones across the country - Prince Harry speaking emotionally about needs of the young at Kensington Palace," British journalist Ranvir Singh shared on Twitter.
Encouraging #onsideyouthzones across the country - Prince Harry speaking emotionally about needs of the young at Kensington Palace. pic.twitter.com/UJXw1V7tYY
— ranvir singh (@ranvir01) June 7, 2018
"Chatting with Prince Harry about mental health, and the pressures faced by young people today," businessman David Price captioned the photo below. "Incredible support from him for the Inspire Youth charity we back in the North West ���� We maaay have also talked about helicopters.. ������ Absolute gentleman x."
A post shared by David Price (@davyprice)
A post shared by Umar Kamani (@umarkamani)
A post shared by Aisha (@aishakamani)
The event was held in Kensington Palace and took place to honor Onside Youth Zones, a charity designed to give young people and people with disabilities a space for them to occupy their bodies and minds with fun activities, learn new skills, and socialize in a safe, positive way, according to its website.
The Duke of Sussex took a moment to praise the organization for its work and highlight the importance of "meeting the needs of young people," according to royal correspondent Omid Scobie.
The Duke of Sussex is telling a large gathering what a massive difference @OnSideYZ can make to this country in the coming years. We're building one in Hammersmith. If you can help, please get in touch. pic.twitter.com/TLBpF6fqZk
— Mark Davies (@markxdavies) June 7, 2018
Harry's wife, the Duchess of Sussex, was not featured in any of the photographs shared on social media, so it's unclear if she was also in attendance. However, the couple will likely both attend the Trooping the Colour ceremony on Saturday, which is held every year in honour of Queen Elizabeth's birthday.
Markle will also make her first joint public engagement with the Queen, without Prince Harry, on June 14. The new Duchess of Sussex will join Her Majesty in officially opening the Mersey Gateway Bridge in Cheshire, opening the Storyhouse Theater in Chester, and attending a lunch at the Chester Town Hall, the royal family website announced Monday.
Via Harper's Bazaar US
From: Harper's BAZAAR US
Another official photograph has been released of Prince Harry and Meghan Markle
Prince Harry and Meghan Markle make their first public appearance together as a couple
Prince Harry and Meghan Markle aren't actually called Harry and Meghan
Prince Harry and Meghan Markle announce their engagement
Prince Harry and Meghan Markle appear at photo call together
Prince Harry releases statement regarding harassment of Meghan Markle


text:
Q: Casting bit data To and From float I have a problem that I want to pack very specific data into specific bits and store them in a float. I already investigated ways of simply packing numbers into floats, but using simple math won't work for what I want because I need to use the full 32 bits to store very specific values.  If it was a 32 bit integer, this would be very easy.
So what I want to do is encode the data as a 32 bit integer and then turn this bit data directly into a float with all the bits remaining the same (unless someone has a better suggestion on how to do it). What languages will allow me to do a conversion like this?  Obviously, not javascript and python because they don't support 32 bit floats. Will C# or C++ do it?
I need to decode the data in a GLSL or HLSL vertex shader.   The shader would, of course, receive the 32 bit float.  Is there an operator that will allow me to turn the float directly to integer with all the same bits instead of an ordinary cast?  Or perhaps some other way to read the bits directly?

UPDATE:  Eric Postpischil showed how to easily do the direct conversion in C in an answer below.  Now I just need to know if there's a way to do a direct conversion from float to int or bit data in a vertex shader.  Can anyone help on that part?

A: You can do this in C with:
#include <stdint.h>

float IntegerToFloat(uint32_t u)
{
    return (union { uint32_t u; float f; }) {u} .f;
}

uint32_t FloatToInteger(float f)
{
    return (union { float f; uint32_t u; }) {f} .u;
}

Naturally, this requires that float be 32 bits in the C implementation, and that uint32_t be a supported type (but you can use another 32-bit integer type if it is not, likely unsigned int). Some of the resulting float values may be NaNs, which might not remain unchanged in certain operations, such as conversion for printing or display and conversion back. Even normal float values will not generally remain unchanged unless they are displayed with sufficient precision and the C implementation uses correct rounding for decimal-to-binary and binary-to-decimal conversions.
So abusing the bits like this is a bad idea unless it is compelled with no alternative.

redpajama_set_name: RedPajamaStackExchange


Whether it's inheritance tax planning, succession planning in the family business, gifting a house deposit, helping to finance home improvements or paying for furniture or a car, financial support from mum and dad is often closely woven into the future plans of newly married or cohabiting couples.
If the parental money has been loaned or given to help a son or daughter purchase a property in joint names with their cohabiting partner, the partner may be entitled to 50% of the property even if they haven't contributed anything. If the son or daughter is married, their spouse may be entitled to a share.
In the case of farming families, buildings and land may have been passed down through generations and matters are further complicated if the business supports the farmer's relatives and their families or where property is owned jointly. We have a lot of experience of working with farming families and our role, whether we are advising a spouse in a divorce or the trustees of a landed estate, will be to achieve the desired outcome for our client whilst protecting the interests of future generations and the viability of the business.
We have seen instances where mum and dad have given their son or daughter land next to their own home to enable them to build their own property. This can be a practical and cost-effective option for the couple starting out together but what if they separate and both want a share of the property? It may have to be sold or mortgaged to release capital for a settlement.
Sometimes parents lend money to cover a major expense such as house renovations, with the intention that it will be repaid at some time in the future. In these situations the arrangement is usually based on trust alone and not documented and it could be argued that it was a gift rather than a loan.
If you are moving in with a cohabiting partner, make sure any parental money is paid into an account in your sole name rather than into a joint bank account. If the money is for a deposit for a house and your partner can't match the deposit consider whether the house should just be in your name or owned in unequal shares.
Cohabitation Agreements and Marital Agreements (pre-nup before marriage and post-nup after marriage) can be drawn up by us for you. These are designed to protect as far as possible any money received from parents or assets acquired before the marriage.
Anyone who doesn't want assets to be shared equally with their partner and spouse in the event of the relationship ending should take legal advice at the earliest opportunity.
If you are a parent wanting to take steps to protect your investment read our advice on safeguarding family money.
To see how we can help you protect your position give us a call today on 01423 594680.


text:
Biografia
Nella sua vita è stato guardia del corpo, buttafuori, esperto lottatore della boxe a pugni nudi, indicato spesso come l'uomo più duro della Gran Bretagna, soprannominato The Guv'nor.
Fra i suoi avversari più noti in incontri di pugilato John McCormack, Johnny Waldron, Roy Shaw.
I suoi interessi economici derivarono anche da alcuni suoi investimenti nell'industria del cinema. Nacque in una zona molto povera e problematica dell'east side London ma, luogo allo stesso tempo, pieno di spirito di comunità. Figlio di Leonard McLean senior che morì quando McLean aveva solo 4 anni. Il padre era membro della Royal Marines nel corso della seconda guerra mondiale. Alla sua morte la madre, Rose, si risposò con un uomo violento, Jim Irwin, che fece ricorso più volte alla violenza contro i figli di lei, al punto che il ragazzo fu ritrovato due volte con la mascella rotta. Spesso il patrigno usava usare violenza contro di lui e i suoi quattro fratelli, anche con l'aiuto di una cintura, ogni volta che gli si parlava davanti.
Come rivelato dallo stesso McLean in un'intervista, Irwin gli fratturò entrambe le gambe a soli 5 anni, la mascella a 6 e, tutte le costole, a 7. L'uomo continuò a usargli una brutale violenza fino all'età di 12 anni.
Irwin è finalmente uscì di scena quando lo zio di McLean lo picchiò per gli abusi che aveva arrecato ai suoi familiari.
Durante la sua adolescenza, McLean fu coinvolto in molti crimini e questo contribuì a trasformarlo in un uomo di quasi un metro e 90 che pesava 127 chilogrammi.
All'età di diciannove anni incontrò Val che diventò in seguito sua moglie. La coppia ebbe due figli, Jamie e Kelly.
Perse la madre all'età di 21 anni e il tragico evento gli causò svariati problemi di alcolismo. Nei mesi a seguire infatti fu visto spesso in moltissimi pubs della zona dove, di sovente, vi faceva scoppiare il caos.
Dopo un incidente in un combattimento clandestino, che lo fece finire in carcere, smise definitivamente di bere e iniziò la sua carriera come buttafuori nei locali nell'east London.
Dall'età di 26 anni si dedicò anche ai combattimenti a mani nude. Negli anni 70 i combattimenti clandestini, in quella zona della città, erano molto popolari.
Il suo primo match nella disciplina fu contro Roy Shaw. McLean Perse il match.
La sconfitta gli provocò un forte spirito di rivalsa che lo porto a chiedere al suo avversario uno spareggio nel 1978. McLean questa volta vinse l'incontro.
Il soprannome di "guv'nor" (il boss, il padrone) gli fu affibbiato quando incontrò per la terza volta Shaw. L'incontro vide prevalere McLean con una forza inarrestabile e devastante. McLean alla fine del match fu udito urlare:"I'm the guv'nor!". All'incontro assisterono più di 30.000 persone in una sfida che assunse oramai una valenza del tutto personale tra i due. Il suo allenatore dell'epoca, Freddy Hill che lo preparò all'incontro, gli insegnò come meglio convogliare la rabbia e gli impartì delle preziose nozioni su come migliorare la sua tecnica di combattimento.
Anni dopo fu coinvolto in un brutto episodio di violenza in cui un uomo, ebbe una accesa discussione con una ragazza in un pub dove McLean lavorava. Quest'ultimo si  fratturò entrambe le mani contro il viso delluomo e gli provocò un morso profondo sulla trachea che lo ridusse in fin di vita.
Il pronto intervento dei medici chirurghi gli salvò la vita e evitò a McLean di entrare per l'ennesima volta in carcere.
Morì a soli 49 anni, dopo aver contratto il cancro ai polmoni, pochi giorni prima del lancio del suo ultimo film, Lock & Stock - Pazzi scatenati, che fu dedicato da Guy Ritchie alla memoria dell'attore.

Filmografia
 Box On (1980)
 Il quinto elemento (Le cinquième élément), regia di Luc Besson (1997)
 Lock & Stock - Pazzi scatenati (Lock, Stock and Two Smoking Barrels), regia di Guy Ritchie (1998)

Opere
Egli ha scritto anche un'autobiografia dove racconta la propria vita di lottatore, fu poi riveduta e pubblicata postuma, intitolata: Lenny McLean e Peter Gerrard, The Guv'nor. Blake Publishing 2003 ISBN 1-85782-570-5

Note

Bibliografia
The Guv'nor: Through the Eyes of Others. Anthony Thomas, Lenny McLean, Valerie McLean. John Blake, 2007.ISBN 978-1-84454-475-2
Lenny McLean the Guv'nor: a tribute. Peter Gerrard. Blake, 2000. ISBN 978-1-85782-397-4

Collegamenti esterni


The John Phillip Immroth Memorial Award, presented annually, honors notable contributions to intellectual freedom and demonstrations of personal courage in defense of freedom of expression.
Established in 1979, upon the death of John Phillip Immroth, this award honors the courage, dedication, and contribution of a living individual, group, or organization who has set the finest kind of example for the defense and furtherance of the principles of intellectual freedom. The award consists of a citation and $500. John Phillip Immroth was a teacher, author, scholar, advocate, and defender of First Amendment rights. He was the founder and first Chair of the Intellectual Freedom Round Table in 1973. His impact on the ideal of intellectual freedom and its practice was great.
Support the award with a $25, $50, $100, or $250 donation to IFRT.
The John Phillip Immroth Memorial Award is sponsored by the Intellectual Freedom Round Table (IFRT) of the American Library Association (ALA). The deadline for nominations is December 1 of each year.
Questions? Call 312-280-4226 or E-mail oif@ala.org.
Donations support IFRT projects: sponsoring Emerging Leaders; networking and continuing education events; promoting core professional values; and awards to honor champions of intellectual freedom, authors, and exemplary chapters or organizations. Please support the hard work of IFRT members with a $25, $50, $100, or $250 donation.


text:
var sqlite3 = require('sqlite3').verbose();
var db = new sqlite3.Database('events.db');

db.serialize(function() {
	db.run("CREATE TABLE IF NOT EXISTS events (time TEXT, remote_ip TEXT, host_ip TEXT, remote_port TEXT, service TEXT, type TEXT, longitude INTEGER, latitude INTEGER, country_name TEXT, city TEXT, username TEXT, password TEXT, description TEXT)");

	//row id isn't returned by default
	 db.all("SELECT * FROM events", function(err, rows){
	 		keys = Object.keys(rows[0]);
	 		console.log(keys.join(',\t'))
	 		for(i = 0; i < rows.length; i++){
	 			console.log(Object.values(rows[i]).join(',\t'));
	 		}
 });

});

redpajama_set_name: RedPajamaGithub


Cache_An elderly woman died in a house fire in Cache tonight. The call for help came in around 7:40 from neighbors. They told firefighters that a 98-year-old woman lived in the home. They discovered her body inside. Investigators say it's possible that the fire burned for some time before anyone noticed. Most of the damage was confined to the interior of the house. The fire marshal is on his way to investigate the cause.


This iPad stand for desktop supports Apple® technology inside a scratch-resistant enclosure. Tablet accessories such as this touchscreen display with a VESA bracket can be bolted onto a flat surface via pre-drilled holes for additional security. This stand for desktop mount is a smart device holder with a small footprint. These touchscreen displays have two panels that are attachable to the bottom of the holder with an option to expose or hide the "home" button. This portable stand with desktop mount tilts and rotates for flexible views at trade shows, in hotel lobbies, and in retail stores.
8.6" x 14.5" x 9.3"
7.5" x 10.0" x 0.6"


For sale Beneteau Oceanis 473 built in 2001 and commissioned in 2002. Lovely blue hull, three cabins layout, genset, washing machine heating, B&G electronics (2017), furling cruising chute, Bimini. Worth a visit.
One single berth in saloon and double convertible berths.


Did you know it was from this Spy Hub in the American Embassy in New Delhi that the double-encrypted Indian Nuclear codes were hacked during the Kargil War?
– Read more about this in GreatGameIndia's explosive book India in Cognitive Dissonance.
Shelley Kasli for GreatGameIndia. For a thorough understanding of how the gathering of information by the East India Company laid the foundations of this hi-tech modern surveillance program read our exclusive research report on the issue Digital India in the Age of Information Warfare published in GreatGameIndia – India's only quarterly magazine on Geopolitics and International Relations.


BillerudKorsnäs has been recognised for its leadership in response to climate change and has been awarded a position on the Climate A-list by CDP. CDP is a non-profit organisation that works to transform the way the world does business, thus preventing damaging climate change.
"It is very rewarding that our work is recognised around the world. This is the second consecutive year that we are included on CDP's Climate A-list; in addition BillerudKorsnäs was earlier this autumn also included in the Dow Jones Sustainability Index Europe. Sustainability is integrated into our business, thus taking a holistic approach, which is key to success. For example, in 2015 we succeeded through systematic efforts reducing our own greenhouse gas emissions by 9%, in addition to this our renewable packaging materials and solutions can contribute positively by replacing fossil materials," says Henrik Essén, Senior Vice President Communication and Sustainability.


text:
Seznam občin departmaja Seine-Saint-Denis zajema 40 občin.

(CAC) Communauté d'agglomération de Clichy-sous-Bois-Montfermeil, ustanovljena leta 2001.
(CAS) Communauté d'agglomération Plaine Commune, ustanovljena leta 2001.

Seine-Saint-Denis


text:
Carnie Wilson Has Band-Over-Bypass
Carnie Wilson was one of the first celebrities to have gastric bypass surgery. Her weight-loss procedure was performed live on the Internet in August of 1999 before 50,000 viewers.
I can only assume that being in the spotlight is difficult even under the best conditions. I also assume that the best conditions are fleeting and people sometimes fail. Carnie Wilson has had her share of falls.
Wilson is as imperfect as the rest of us, although her imperfections are open to public scrutiny. Many celebrities are tied to similar circumstances. I suspect they were at least partially aware of the price of fame.
Many people dislike celebrity at any given moment. Carnie Wilson is a celebrity. Her struggles with her weight are well-publicized, and the critiques have sometimes been harsh. It must be difficult and hurtful, and I admire her fortitude.
The Need for Weight-Loss Surgery
Carnie Wilson weighed 300 pounds prior to her gastric bypass surgery. She was pre-diabetic, had slipped discs in her back, and suffered from chronic headaches. Her liver was enlarged and toxic, and she had sleep apnea. Her cholesterol and blood pressure were elevated. Dieting changed nothing.
Wilson would lose half of her body weight following bariatric surgery, about 150 pounds.
She advocated for weight-loss surgery after her operation and helped educate the public about the procedure.
Carnie Wilson Has Second Surgery
Wilson publicly acknowledged that maintaining an appropriate weight is a struggle and that she had gained back two-thirds of her weight. Her blood-sugar levels began to rise, and fear of diabetes prompted her decision to have Lap-Band surgery. Commonly referred to as "band-over-bypass" the LAP-Band is used to further restrict the volume of food that the gastric bypass pouch is able to hold.
You may view a Lap-Band surgery being performed on YouTube.
Wilson cites the birth of her two children as contributing to her weight gain.
Obesity is a Disease
Carnie Wilson has been subject to criticism both before and after her surgeries. Some are critical because they have stereotypical views about obesity and think that those who are obese do not have willpower and are lazy. Many cannot accept obesity as an illness.
Obesity is recognized as a disease by such medical associations as the American Society of Bariatric Physicians (ASBP), the American Medical Association (AMA), and the North American Association for the Study of Obesity (NAASO). Even the Internal Revenue Service (IRS) agrees that obesity is a disease.
Obesity is a chronic, metabolic, and progressive illness with a genetic predisposition. The scientific community believes there are oevr 1,000 genes related to weight. About 200 have been discovered.
Although Bariatric surgery has significantly improved the lives and health of many people, there is no magic in the procedure. It should not be viewed as an alternative to the lifestyle changes that are necessary such as proper nutrition and exercise. Bariatric surgery is a tool that can help people become more successful in changing their lifestyles.
Sep 30, 2015 My Bariatric Life
September 30, 2015	Bariatric, Bariatric Success Stories, Bariatric Surgery, Inspirationband-over-bypass, bariatric, bariatric surgery, carnie wilson, gastric bypass, LAP-Band, obesity, revisions, weight gain, weight loss surgery8,894
Mark Sisson Primal Cookbook Diet ReviewBento Box Lunch Solutions after Bariatrics
Guide to Weight Loss Surgery Options
Good for Your Gut Foods to Make You Feel Amazing
My Acne Facial, Constipation and Hormones


text:
Yahoo Style UK
Woman who saved £10,000 during first two lockdowns shares her tips for stashing the cash
Marie Claire Dorking
Amy De Keyzer has managed to save £10,000 during the pandemic. (Caters)
A woman who managed to save £10,000 during the first two national lockdowns has revealed her money saving secrets.
In March 2020, when the first lockdown hit England, Amy De-Keyzer, 32, from Horsham, West Sussex, set herself the challenge of saving more money.
By the time the first set of coronavirus restrictions were eased the communications professional had managed to put away £5,000.
But De-Keyzer wanted to challenge herself to save even more and has managed to rake in ten thousand pounds worth of savings by cutting back on her spending during the pandemic.
Now she's hoping to increase her saving stash further during the third national lockdown, as she and her husband are saving up to complete a big renovation project on a new house.
"Another lockdown is a blow, but I'm trying to see the positive side and look at it as another opportunity to save," she says.
"I'm hoping to save around one thousand pounds in the next six weeks."
Some of the super saver's tricks for putting away more money include cutting back on her spending by freezing her cinema membership card while venues were closed; switching energy providers; using supermarket coupons and cutting her weekly spend on fuel as she began working from home.
Amy De-Keyzer saved money by upcycling old furniture. (Caters)
De-Keyzer also began upcycling old furniture around the house and selling it on Facebook marketplace, which brought in extra cash.
"Lockdown has meant spending less on stuff that you enjoy; it's just a product of the situation we find ourselves in," she says.
"So, I have saved a lot of money in fuel for my car, going out for dinner, my cinema membership card and just all the stuff that we haven't been able to do."
Watch: Generation Z is more savvy when it comes to saving money.
In terms of tricks and tips, De-Keyzer didn't do anything too out-there. She simply looked at her outgoings, worked out where she could cut back, and made saving a priority.
"I've been moving money into my savings account every month because it seemed a sensible thing to do," she explains.
"At the beginning of the month when I get paid, I will always move a set amount into my savings and then anything extra I have left at the end of the month, I tend to move over as well.
"I see my savings account as completely separate from my current account and hate taking money out of there; it's good to have a target in mind."
The couple also saved money by repurposing unloved items and doing jobs themselves instead of paying a professional.
"We did a garden project over the summer and because we had a lot of time on our hands, we repurposed things and did a lot of the stuff ourselves rather than paying someone else to do it," she says.
Amy De-Keyzer saved £10,000 by cutting back on her spending during the pandemic. (Caters)
The savvy saver is now an advocate for shopping around as a way to save extra money.
"Normally, we can't be bothered to shop around energy providers because it seems like quite a boring task but we managed to make a huge saving by doing so," she explains.
And she recommends others do the same.
"Look at your bills and see if you could save – we checked our car insurance, energy providers, WIFI and it doesn't take long at all, but most people put it off."
Working from home has helped De-Keyzer cut back on unnecessary spending during the week.
"When you're in the office, you'll quickly pop to the shop for snacks or go and get a coffee," she says.
"You'll go for drinks after work or go out with colleagues for lunch and it's cutting back on things like that that have really helped."
She now wants to encourage other people to try to use lockdown as an opportunity to bank away some cash.
"I've always been quite good at saving but this whole situation has really helped me save more."
Additional reporting Caters.
Watch: TikTok money saving hack.
Sunday Essay: How to make a taxpayer's day


text:
Q: Java formatting something of variable size with Formatter So I'm trying to write a toString method that prints a representation of a variable-sized Board object with size N x N, so for example for N = 6 the representation would look like this:
===
    2r -- 2r 2r -- 2b
    -- -- 2r -- 3r --
    2r 3r 2r 3r -- 2b
    3r 1r 3r 2r 2r 2b
    2b 4r 3r 1r 3r 2b
    2b 2b 3b 2r 3b 1b
===

Every "Square" on this board is stored in a Square[]. My question is, since the size of this board is variable, how would I write a format string to be used by Formatter.format?
This is what I have so far, given squares is my Square[]:
/** Returns my dumped representation. */
@Override
public String toString() {
    Formatter out = new Formatter();
    String format = "Something here";
    out.format(format, squares);
    return out.toString();
}

I was thinking of trying to use a couple for loops and printing it out line by line, square by square, but I'm hoping theres a cleaner way to do this.

A: I would try to use a StringBuilder instead a Formatter:
final StringBuilder sb = new StringBuilder();
final int n = (int) Math.sqrt(squares.length);
for (int row = 0; row < n; row++) {
    for (int col = 0; col < n; col++) {
        final int offset = row * n + col;
        final Square square = squares[offset];
        sb.append(square.toString())

        final boolean lastCol = col == (n - 1);
        sb.append(lastCol ? "\n" : " ");
    }
}
return sb.toString();


text:
The Group Areas Act Essay - :DistrictSix.
Forced Removals Under the Group Area's Act: District Six The Group Areas Act No. 41 was a piece of Apartheid legislation officially commenced on July 7 th, 1950. This act, along with its subsequent amendments, gave the government the power to divide urban areas into separate zones, segregated by race.
The Group Areas Act was fashioned as the "cornerstone" of Apartheid policy and aimed to eliminate mixed neighbourhoods in favour of racially segregated ones which would allow South Africans to develop separately (South African Institute for Race Relations, 1950: 26).
No. 41 of 1950 40 THE GROUP AREAS ACT.
B No. 5 - GROUP AREAS ACT: This 22nd Conference of the South Afrioan Indian Congress held at the Gandhi Hall, Johannesburg on 19th, 20th and 21st October, 1956 reiterates Its total rejection of the Group Areas Aot and demands its immediate repeal.The 'Group Areas Act' (1950) separated blacks, coloured's and whites into distinct areas. It sought to keep blacks inferior and place them into sub-standard areas. In order to separate the races, the Government needed to know the race to which people belonged. To do this, the 'Population Registration Act' was introduced in the same year.The purpose of the Group Areas Act of 1950 was to legally establish apartheid in South Africa. It set up segregated residential and commercial districts in urban areas throughout the country. It.
They then continued to control that population with the Group Area Act, facilitating control over the black urban population. This act attempted to hamper organization among the oppressed urban working class. Also, the segregated townships were placed on the outskirts of cities.After a more rigorous implementation of the Group Areas Act in 1950 a new separation between ethnic groups such as South Sotho's, Xhosas and Tswana's were formed. This formed part of the greater sectored model of Apartheid. Physical buffer such as the railway line and roads further strengthen separate development outward along these barriers.
The People Wept; being a brief account of the origin, contents, and application of that unjust law of the union of South Africa known as The Group Areas Act of 1950 (since consolidated as Act No. 77 of 1957) by Paton, Alan and a great selection of related books, art and collectibles available now at AbeBooks.com.
The Group Areas Act of 1950 was the core document of apartheid in South Africa because it initiated physical separation between races. Different racial groups were allowed to live in specifically marked areas and were prohibited from moving to other places. As a result, thousands of Africans were forcibly removed from rural areas, which were proclaimed "white," to racially segregated areas.
There were still issues of displacement for people due to the Group Areas Act. This had resulted in a break down in the economic industry. The new government was left with subsequent debts from the previous regime, huge unemployment rates, non-existent social welfare support, high level of domestic violence, low levels of education and high drop out rates at schools.
The Government Law Advisers soon after found that the proclamation said the exact opposite, and the Group Areas Board became the laughing stock of the Civil Service. Instead of withdrawing the proclamation and issuing another, the Board tried to save face by amending the Act, quite unnecessarily, in 1955.
There were different kind of legislations used to abduct the non-white from their pride and dignity. This essay underlines the policies of apartheid; the "Guetto Act", the economic and racial legislation, Prohibition of mixed marriages Act, Group areas act, educational legislation (Bantu Act), amongst all.
Apartheid Group Areas Act The act was designed to restrict the black or colored race group to its own residential and trading area; To control the purchase or occupation of land or dwellings in a specified area under the Act. Indians and coloreds were uprooted from homes at enormous cost to.
Safe, very safe. You live d in an area roughly populated by people of the same culture. You could safely walk down the street at night. People adhered to similar practice s, ie did not slaughter animals in your bank yard. Did not build shack in th.
The Presidency National Party and the legacy of Empire, the ANC, Apartheid laws, Group Areas Act. The Constitution, Changing levels of confidence, anti- Communism, the New Deal Causation essay on the success of the National Party. Source based essay on the Group Areas Act.
The White House Essay Otherness is the act of one group or individual viewing another as inferior because of apparent differences, often to bestow feelings of self-importance on themselves. Otherness can be found in a variety of forms.
Definition of Group Areas Act in the Definitions.net dictionary. Meaning of Group Areas Act. What does Group Areas Act mean? Information and translations of Group Areas Act in the most comprehensive dictionary definitions resource on the web.
Watch the video for Group Areas Act from Lucky Dube's House of Exile for free, and see the artwork, lyrics and similar artists.
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text:
Toronto power supply vulnerable, 2007 report warned
By James Armstrong Global News
Updated July 10, 2013 5:55 pm
TORONTO – Six years before a record-setting rainstorm left hundreds of thousands of Torontonians in the dark, experts warned the region was vulnerable to just this sort of power outage.
West-end residents endured days of rolling blackouts after Monday's rainstorm knocked two key hydro distribution centres offline.
And a report written in 2007 and obtained by Global News warns of exactly that, because not enough power is generated within the region.
"The ability of the existing infrastructure to supply these [west and north GTA] areas is expected to fall short by 2015," the report reads.
On Monday, an unprecedented storm dropped 126 mm of rain on the city, breaking the previous record of 121 mm set in October 1954 during Hurricane Hazel.
Related: Power restored to Toronto Hydro two days after unprecedented storm.
That storm knocked out the transmission stations at Richview and Manby – both singled out in the 2007 report as being particularly at risk.
"Extraordinary events or major failures on the transmission system could lead to inadequate supply capacity or voltage stability issues. The risk of such events is significantly reduced with internal generation capacity."
The report recommends building new gas generating power plants in the southwest part of the GTA.
But those two plants, which were to be located in Oakville and Mississauga, were cancelled prior to the 2011 election by the Ontario Liberal government.
"We had no serious political debate. All the parties lined up on getting rid of the plants, and so the power plants just got thrown to the sharks," said Tom Adams, a Toronto-based energy consultant.
Ontario produces more than enough power to meet Toronto's demands. The challenge "really is around the capability to bring that power into Toronto," said Terry Young, VP of Corporate and Employee Relations at the Independent Electricity System Operator.
Related: Watch a timelapse of Monday's storm blowing across Toronto's skyline.
Toronto has two main corridors, each with two facilities, that feed power from Ontario's generating grid into the city. Two of those facilities are in the east at Cherrywood and Leaside and two are in the west at Richview and Manby.
"Two of the major transformer stations [Richview and Manby] that actually do bring the power into the city were flooded out" Monday, Young said. "So you no longer had that major network, if you will, in order to bring that power in."
New York City requires at least 80 per cent of its energy be generated inside of the city's borders to protect against problems created by distant distribution facilities.
But there's no such requirement in Ontario.
Adams said that plants in Mississauga and Oakville were supposed to take the place of the shuttered Lakeview coal-fired plant and serve as important backup power stations. The 2007 report states these gas-fired plants would help relieve the Richview and Manby transformers, which Adams says are "so overstretched that they can't be taken out of service to be maintained."
"Politics intervened. And those critical backup power stations were moved," he said. "One to Napanee and the other one to Sarnia. Which is ridiculous."
The 2007 report notes that power generation within the region has declined rapidly since 1985.
"With less internal generation," the report reads, "The GTA has become more dependent on the transmission system to import power into the GTA."
– With files from Jackson Proskow
Toronto flood
© 2013 Shaw Media


The Art of Cookery: Courgettes - Italian Courgettes from Tuscan Cooking.
Cut the courgettes into sticks about five centimetres long. Bring the water and vinegar to the boil and plunge in the chopped courgettes. Cook for fifteen minutes, drain and leave in the colander for twelve hours.
Put into a glass preserving bottle, interspersed with cloves of garlic, fresh rosemary leaves and a little salt. Cover with olive oil and close the bottle firmly.


PACIFIC PALISADES, Calif – Amanda McDowell and Maya Johansson continued their run in the singles bracket while Whitney McCray and Kristi Miller progressed in the doubles bracket on day two of the main draw at the ITA All-American Championships, which is being played at the Riviera Country Club in Pacific Palisades, Calif.
"It was another great day at the Riviera," head coach Bryan Shelton said. "Maya won back-to-back again today, and has now won nine-straight matches in this tournament. I thought it was great that she was the only freshman to make it to the main draw, but she's playing with heart on the court and is leaving everything she has out there.
"Amanda's match was amazing. To win like she did under the lights was unbelievable.
McDowell and Johansson will join Clemson's Ani Mijacika and Cal's Suzi Babos in the semifinals of the singles tournament, with McDowell and Babos squaring off while Johansson meets Mijacika Saturday afternoon. Babos is the only remaining seeded singles player in the tournament after five of the top eight seeds fell in the first round and another two were defeated Friday afternoon.
Johansson knocked off Baylor's Lenka Broosova, 6-2, 6-4, to begin the day before winning 12 of her last 14 games against UCLA's Riza Zalameda in the quarterfinals to win 3-6, 6-0, 6-2. With her two singles wins Friday, the Yellow Jacket freshman moved to 12-0 on the season.
McDowell squared off against Florida's Csilla Borsanyi in the round of 16, winning in straight sets, 6-3, 6-3, to set up a quarterfinal match with Miami's Laura Vallverdu in the afternoon. After dropping a hard-fought first set to the Miami standout, the Yellow Jacket sophomore won her second set, 7-5, before battling for an 11-9 tiebreaker victory in the third and final set to win 5-7, 7-5, 7-6 (9).
Earlier in the day, Tech's senior duo of Miller and McCray stopped the Northwestern tandem of Lauren Liu and Samantha Murray, 8-6, to continue their run in the doubles tournament. The Yellow Jackets will face LSU's Megan Falcon and Hannah Robinson in the semifinals Saturday morning.
After falling in her first round match Thursday, Miller posted a straight-set singles win against UCLA's Tracy Lin to advance to the semifinals of the consolation bracket, which will be played Saturday at 10 a.m. PT.
Saturday's matches will be broadcast live at www.RadioTennis.com with Ken Thomas providing the point-by-point commentary starting at 10 am PT.
Finals for both the doubles and singles brackets will be played Sunday.


text:
extern double BinaryTreeVersionNumber;

/// Project version string for BinaryTree.
extern const unsigned char BinaryTreeVersionString[];