Brian Borkowski, pictured bartending, bought Vino Etc. and started running the Wisconsin Avenue wine bar on Jan. 1.
OCONOMOWOC — Vino Etc. is under new ownership as of Jan. 1 with former Vino Etc. bartender Brian Borkowski taking over.
Borkowski said he has lived in Oconomowoc for 15 years, and after being a high school coach at University Lake School and Lake County Lutheran High School, he stepped down when his son got to high school.
Borkowski said he wants to be famous for his customer service. "You can't do everything, but I do want to react, innovate and change," he said.
In his four years of bartending at Vino Etc., 120 E. Wisconsin Ave., Borkowski said he knows the clientele and what they are looking for.
Vino Etc. offers a wine club where members get a loyalty card and special discounts.
It was expanded to a bourbon club with the same benefits, Borkowski said.
Customers had said to Borkowski that they didn't come in because they wanted to watch sports games while having a glass of wine, but Vino Etc., didn't have a TV.
So Borkowski added a TV to watch, along with a revamped menu and a slew of specialty drinks since taking over.
"My wife and I created our own spin on an old fashioned, which is an old fashioned with pinot noir with either bourbon or brandy," he said.
Borkowski said Vino Etc. is known for its wine, but wants people to know the wine bar is also stocked as a full bar.
"We have slew of bourbons and vodkas," Borkowski said. "We're famous for wine, but we are a full bar.


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Good news Kung Fu Panda fans. Po is back in a new trailer. This time it's full of action and training montages. The thing all good kung fu movies need. Possibly not the way it looks in this movie unfortunately. Just keep an eye out for Master Chicken. He's a chicken if you miss him!
Not only do we get the brand new trailer but a brand new poster. This time it's Po showing the young Pandas how to fight. I wonder how that turned out!


text:
\section{Introduction}
Since H.B.G. Casimir wrote his seminal paper \cite{Cas48} proposing that two uncharged metallic plates should attract in vacuum due to quantum fluctuations still little is known of how to revert the sign of the force and obtain repulsion or levitation. The generalization of the theory to include dielectric bodies \cite{DLP61} has made it possible to achieve, very recently, repulsion with test bodies immersed in a dielectric fluid \cite{MCP09}. However, achieving repulsion in vacuum, which would have important consequences for device applications \cite{KMM09,BKMM09}, is still to be experimentally tested. Theoretically, there have been several proposals to achieve such situation. The first proposal considered magnetic versus non-magnetic situations \cite{B74} and more recent proposals include the use of metamaterials \cite{RDM06,LP07,ZZK09a} and geometry to induce repulsive scenarios \cite{LMR10}. Importantly, it has also been shown that for general dielectric-dielectric situations, there is no repulsive behavior in vacuum \cite{RK09}. In a recent paper \cite{GC10}, two of us suggested that repulsive behavior could be achieved by using topological insulators \cite{Moore10,HQW08,HXW09,HK10}. The topological nature of these materials \cite{QHZ08,EMB09} provides a magnetoelectric term modifying the response to an external electromagnetic field, which can then cause the Casimir effect to reverse sign at short distances and remain attractive at large distances\cite{GC10}. Consequently, at an intermediate distance $d_{eq}$, the Casimir force vanishes and a stable configuration is possible.\\
In this work, we aim to include the effect of temperature and uniaxial anisotropy to this behavior, two relevant factors in experimental situations. It is well known by know that anisotropy can modify the Casimir force by changing the form of the reflection coefficients \cite{BKMM09}, and has been studied in the context of repulsive interactions \cite{DLL08}, even including the effect of temperature \cite{RDM08}. In the present paper we address the question of whether uniaxial anisotropy and temperature can enhance or destroy the repulsive behavior in the context of topological insulators, and in what cases can this occur. To achieve this goal we derive the reflection coefficients for a generic anisotropic topological insulator, a result which to our knowledge is absent in the topological insulator literature. With the help of these, we find that low temperatures favor the repulsive behavior and we determine that enhancing uniaxial anisotropy in the direction parallel to the optical axis also acts to increase repulsion.\\
To our knowledge, precise optical characterization of these materials is still lacking, and thus it remains an open question if real materials are to show repulsion at these distances. Nevertheless, throughout the paper, we use choices of parameters which can be relevant for topological insulators such as TlBiSe$_2$\cite{Chen10} (see also concluding paragraph in Ref.\cite{GC10}) which are mainly low dielectric permeability at zero frequency $\epsilon(0)$ and small magnetoelectric polarizability $\theta$. We do not restrict the study only to these values but explore other regions of parameters for completeness.\\
The work is structured as follows. Section \ref{sec:T=0} is devoted to review the formalism and notation on which we rely on. To do so, we will briefly review the isotropic case at zero temperature ($T=0$) discussed in Ref. \cite{GC10}, to which we will add the dependence of the minimum with the topological magnetoelectric polarizability, not discussed in Ref. \cite{GC10}. Details of the proof of the existence of repulsion are left for appendix \ref{App:Minimum}. In section \ref{sec:Tneq0} we will study the effect of temperature on the Casimir energy as a function of distance, both analytically and numerically. We will also discuss the position of the minimum as a function of temperature and topological magnetoelectric polarizability $\theta$. Details of the analytical results can be found in appendix \ref{App:class}. In section \ref{sec:uniaxial} we will discuss the effect of uniaxial anisotropy on the Casimir energy at $T=0$. First, we will explicitly write the Fresnel coefficients for this case, leaving the details of the derivation for appendix \ref{App:coef}. In the remaining part of this section we will consider different values for the relevant parameters and discuss their effect on the position of the minimum. Finally, in section \ref{sec:uniaxialandtemp} we will present the results for the case of uniaxially anisotropic topological insulator at $T\neq0$ to end with section \ref{sec:conc}, which includes a summary of results and some concluding remarks regarding real systems.\\
We emphasize that the numerical results presented in this paper explore regions of parameters without any restricting assumption other than positive energy condition inherent to magnetoelectric couplings, discussed in section \ref{sec:Tneq0}.B. On the other hand, in order to derive analytical results, some feasible assumptions are to be considered, such as small magnetoelectric coupling, all of which apply only to the results in appendix \ref{App:class}, and hence will be discussed in the mentioned appendix.

\section{\label{sec:T=0}Casimir-Lifshitz force between topological insulators at $T=0$}

It is well known from different approaches, that the Casimir energy density stored by two dielectric parallel plates (labeled $1$ and $2$) of area $A$, separated by a distance $d$, at zero temperature ($T=0$) can be written as\cite{DLP61,Reyn91,RE09,BKMM09}:
\begin{equation}
\label{CasimirEnergy}
\frac{E_{c}(d)}{A\hbar} = \int_0^{\infty} \hspace{-1pt} \frac{d\xi}{2\pi} \int \frac{d^2 {\bf k}_{\|}}{(2\pi)^2} \log \det \left[1 - {\bf R}_1 \cdot {\bf R}_2 e^{-2 k_3 d}\right] ,
\end{equation}
where $k_3=\sqrt{\bm{k}^{2}_{\|}+ \xi^2/c^2}$ is the wave vector perpendicular to the plates, $\bm{k}_{\|}$ is the vector parallel to the plates and $\xi$ is the imaginary frequency defined as $\omega = i\xi$. The matrices ${\bf R}_{1,2}$  are $2\times2$ reflection matrices containing the Fresnel coefficients such that:
\begin{eqnarray}
\label{eq:ReflectionMatrices}
{\bf R} = \left[
\begin{array}{cc}
   R_{s,s} (i \xi, {\bf k}_{\|}) &  R_{s,p} (i \xi, {\bf k}_{\|}) \\
  R_{p,s} (i\xi, {\bf k}_{\|}) &  R_{p,p} (i \xi, {\bf k}_{\|})
\end{array} \right] ,
\end{eqnarray}
where $R_{i,j}$ describes the reflection amplitude of an incident wave with polarization $i$ which is reflected with polarization $j$. The label $s$ ($p$), equivalent to $TE$ ($TM$) modes, describes parallel (perpendicular) polarization of the electric field with respect to the plane of incidence. The Casimir force per unit area on the plates is obtained by differentiating expression (\ref{CasimirEnergy}): $F=-\partial_{d}E_{c}(d)$. A negative (positive) force, or equivalently a positive (negative) slope of $E_{c}(d)$, corresponds to attraction (repulsion) of the plates.\\
In order to calculate the Casimir energy one needs to compute the reflection coefficients. These coefficients relate the amplitude of the incident and reflected electric fields for different polarizations. Since the normal components of $\bm{D}$ and $\bm{B}$ and tangential components of $\bm{E}$ and $\bm{H}$ must be continuous along the interface, one can obtain the reflection amplitudes by solving Maxwell's equations at each side and then imposing the mentioned matching conditions for the fields (see below).

\begin{figure}
\includegraphics[scale=0.2]{TIcas}
\caption{\label{Fig:plates}(color online)Topological insulating plates separated by a distance $d$ covered with a thin ferromagnetic layer of thickness $l<<d$ (not to scale). Changing the sign of the magnetization of one of the plates (parallel or antiparallel to the surface normal) is equivalent to changing the sign of (either) $\theta_{1,2}$.}
\end{figure}

\subsection{Topological insulators: The model}

Following Ref.\cite{GC10} we will consider a Casimir system composed by two topological insulator plates separated by a distance $d$, shown in Fig.\ref{Fig:plates}. The electromagnetic response of three dimensional topological insulators, which determines the reflection coefficients, is governed by the lagrangean:
\begin{eqnarray}\label{eq:lagrangean}
\mathcal{L} = \mathcal{L}_{0} + \mathcal{L}_{\theta} = \left(\bm{E}\cdot\bm{D}+\bm{B}\cdot\bm{H}\right)
\end{eqnarray}
with the difference that now the constitutive relations for the electric displacement field $\bf{D}$ and the magnetic field $\bf{H}$ are given by:

\begin{eqnarray}\label{eq:D}
D_{i} &=& \epsilon_{ij}E_{j}+\dfrac{\alpha\theta}{\pi}B_{i}\\
\label{eq:H}
H_{i} &=& (\mu)^{-1}_{ij}B_{j}-\dfrac{\alpha\theta}{\pi}E_{i}.
\end{eqnarray}

The first term of each constitutive equation is the usual electromagnetic term defined in terms of the dielectric function $\epsilon(\omega)$ and magnetic susceptibility $\mu(\omega)$, giving rise to the ordinary electromagnetic term in the lagrangean \eqref{eq:lagrangean} which we label $\mathcal{L}_0$. We restrict ourselves to non magnetic topological insulators so $\mu=1$.  The second term in each constitutive equation is a non trivial axionic \cite{Wilczek87} or topological magnetoelectric term \cite{QHZ08,EMB09} which gives rise to a topological $\mathcal{L}_{\theta}$ term in the lagrangean. Time reversal symmetry indicates that $\theta=0,\pi$ (mod $2\pi$) being $\theta=\pi$ the case for topological insulators and $\theta=0$ the case for trivial insulators.\\
When the boundary is included, the action corresponding to the lagrangean \eqref{eq:lagrangean}, $S_0+S_{\theta}$, is a fair description of the topological insulator only when a time reversal breaking perturbation is induced on the surface to gap the surface states\cite{QHZ08}. Along the lines of similar situations \cite{QHZ08,QLZZ09,GC10}, in this work we consider that the time reversal perturbation is a magnetic coating of small thickness $l<<d$ ($d$ will be of the order of $\mu$m) which gaps the surface states. In the described situation, $\theta$ is quantized in odd integer values of $\pi$ such that:

\begin{eqnarray}
\theta = (2n + 1)\pi ,
\end{eqnarray}

where $n \in \mathbb{Z}$, determined by the nature of the coating, but independent of the absolute value of the magnetization of the coating. Positive or negative values of $\theta$ are related to different signs of the magnetization on the surface \cite{QLZZ09}, which we consider is perpendicular to the plane of the plates. Each topological insulator plate is characterized by the frequency dependent dielectric function $\epsilon(\omega)$ and the quantized magnetoelectric term $\theta$. Being a topological contribution, $\theta$ is defined in the bulk as a constant whenever the bulk Brillouin zone is defined \cite{EMB09}. Nevertheless, at the surface, the effective action must be valid as long as the condition $l<<d$ is fulfilled, where magnetic effects from the covering magnetic layer could renormalize its value, and the system should be treated as a layered system. We henceforth assume that this is not the case and consider only the region where $l<<d$ (nm $<< \mu$m in practical terms). \\
The parasitic magnetic forces between the magnetic layers can be estimated following Ref.\cite{Bruno02}. The dipole-dipole interaction is of the order of attoN at distances of 50 nm and the magnetic Casimir force\cite{Bruno02} is $\sim 1 fN$. Since we will be dealing with distances of the order of $\mu$m the magnetic forces will be even smaller compared to the Casimir force that is of the order of $p$N\cite{GC10}. Thus, we neglect the parasitic magnetic interactions, and focus only on the Casimir force experienced by the plates.

\subsection{Results for isotropic topological insulator plates at $T=0$}

In this section we review for completeness the case of two isotropic topological insulator plates discussed in Ref.\cite{GC10} and extend some of the results. The topological part $S_{\theta}$ in the action does not modify Maxwell's equations as long as the constituent relations are changed according to \ref{eq:D} and \ref{eq:H}, taken at this stage to be isotropic.\\
From these, we can obtain the reflection matrices \eqref{eq:ReflectionMatrices} by imposing the continuity of the tangential component of $\bf{H}$ and the normal component of $\bf{D}$. For a plate described by the optical responses $\theta_{i}$ and $\epsilon_{i}(\omega)$ immersed in vacuum the reflection matrices are given by \cite{Obu09,CY09}:

\begin{widetext}
\begin{equation}
\label{eq:ReflectionMatricesTIcomplete}
{\bf R}_i = \dfrac{1}{\Delta}\left(
\begin{array}{cc}
  1-n^2_{i}-\bar{\alpha}_{i}^2 + n_{i}\chi_{-} &  2 \bar{\alpha}_{i} \\
  2\bar{\alpha}_{i} & -1+n^2_{i}+\bar{\alpha}_{i}^2 + n_{i}\chi_{-}
\end{array} \right),
\end{equation}
\end{widetext}

where $i=1,2$ labels each plate, $\bar{\alpha}_{i}=\frac{\alpha\theta_{i}}{\pi}$, $\alpha$ is the fine structure constant ($\alpha = \frac{e^2}{\hbar c}$), $n_i = \sqrt{\epsilon_{i}(\omega)}$ is the refractive index of each plate, $\Delta = 1+n^2_{i}+\bar{\alpha}_{i}^2 + n_{i}\chi_{+}$ and:

\begin{eqnarray}
\label{eq:Xipm}
 \chi_{\pm}=
 \dfrac{\xi^2+\mathbf{k}_{\|}^2 \pm \left(\xi^2 + \frac{\mathbf{k}_{\|}^2}{n_{i}^2}\right)}{\sqrt{\left(\xi^2 + \mathbf{k}_{\|}^2\right)\left(\xi^2 + \frac{\mathbf{k}_{\|}^2}{n_{i}^2}\right)}}.
\end{eqnarray}

It is possible to show that when $\bar{\alpha}=0$ and after a little algebra, these coefficients reduce to the ordinary Fresnel coefficients for a dielectric-dielectric interface \cite{Born99}. By its definition, $\Delta$ is always positive and the off-diagonal terms have a an overall sign governed by the sign of $\theta_{i}$. \\
Introducing these matrices in \eqref{CasimirEnergy} and assuming that both topological insulators are described by an oscillator model of the form:

\begin{equation}\label{eq:phendiel}
\epsilon(i\xi)=1+\sum_{i}\dfrac{\omega_{e,i}^2}{\xi^2+\omega^2_{R,i}+\gamma_{R,i}\xi},
\end{equation}

it was shown\cite{GC10} that two different situations could arise: 1) when the topological terms had the same signs, i.e. $\mathrm{sgn}(\theta_{1})=\mathrm{sgn}(\theta_{2})$ the Casimir force was attractive for all distances, and 2) when the signs were opposite $\mathrm{sgn}(\theta_{1})=-\mathrm{sgn}(\theta_{2})$, it was shown both analytically and numerically that a repulsive region at small distances appeared. At large distances, attraction was recovered and the two regimes were separated by a minimum in the Casimir energy; an equilibrium point. The dependence of the minimum was studied for a one oscillator model, showing that the repulsive behavior was favored by reducing the ratio $\frac{\omega_{e}}{\omega_{R}}$. A detailed version of the proof of the existence of a minimum, together with the analytic analysis of the large and short distances limits of the Casimir energy are given in appendix \ref{App:Minimum}.

\begin{figure*}
\begin{minipage}{.49\linewidth}
\includegraphics[scale=0.47]{Fig2a}
(a)
\end{minipage}
\begin{minipage}{.49\linewidth}
\includegraphics[scale=0.47]{Fig2b}
(b)
\end{minipage}
\caption{\label{deqvstheta}(color online)(a) $\bar{d}_{eq}$ as a function of $\theta_{1}$ for different values of $\theta_{2}$ ranging from $\pi$ to $5\pi$. The solid blue line represents $\bar{d}_{eq}\propto |\theta_{1}\theta_{2}|$.(b) $\bar{d}_{eq}$ as a function of $\theta \equiv \theta_{1}=-\theta_{2}$ (black curve with dots). The behavior deviates from $\theta^2$ (bottom curve red) reasonable for small $\theta$. Beyond $\theta=17\pi$ the equilibrium point is lost (see text). For both figures the remaining parameters of the model where fixed to $\frac{\omega_{e}}{\omega_{R}}=0.45$}
\end{figure*}

To end this section we complete the analysis made in Ref.\cite{GC10} by studying the explicit dependence of the position of the equilibrium point ($d_{eq}$) with $\theta_{1}$ and $\theta_{2}$. We define for convenience the adimensional distance $\bar{d} \equiv \frac{\omega_{R}}{c}d$. Whenever the condition $\mathrm{sgn}(\theta_{1})=-\mathrm{sgn}(\theta_{2})$ is satisfied, it is easy to study numerically the dependence of $\bar{d}_{\mathrm{eq}}$, the equilibrium position as a function of both $\theta_{1,2}$. The analysis is shown in Fig.\ref{deqvstheta}. In Fig.\ref{deqvstheta}(a) we plot $\bar{d}_{\mathrm{eq}}$, against $\theta_{1}$ for different values of $\theta_{2}$ ranging from $\pi$ to $5\pi$. A numerical fit indicates that for small magnetoelectric couplings the dependence is given by:

\begin{eqnarray}\label{deqproptheta}
\bar{d}_{eq}\propto |\theta_{1}\theta_{2}|.
\end{eqnarray}

For higher magnetoelectric couplings, the behavior deviates from the simple $\theta^2$ law. This is shown in Fig.\ref{deqvstheta}(b) where we plot $\theta\equiv \theta_{1}=-\theta_{2}$. For high values of $\theta$ the equilibrium position grows faster to larger distances. Beyond a critical value, the magnetoelectric part of the reflection coefficients overwhelms the ordinary dielectric part giving rise to purely repulsive behavior and the equilibrium position disappears which is analogous to the $\epsilon(0)\to 1$ limit discussed in Ref. \cite{GC10}. The inclusion of temperature will modify further \eqref{deqproptheta}, as shown in the next section.\\
As a final comment for this section we mention that the obtained dependence of the minimum with $\theta$ suggests that an analytic way of deriving this result might be possible, especially in the case where $\theta_{1}=-\theta_{2}$. Nevertheless, the derivation of this result is not transparent from this formalism, although other formalisms\cite{RE09} can shed more light to the issue.

\section{\label{sec:Tneq0}Casimir-Lifshitz force between isotropic topological insulators at $T\neq0$}

In this section we include the effect of temperature for isotropic plates and we discuss how the repulsive behavior can be affected by changes in temperature.

\subsection{Inclusion of finite temperature effects}

To take into account finite temperature effects within the Lifshitz theory one must assume that the system is in thermal equilibrium. As a first step, the formal replacement \cite{BKMM09,RE09}:

\begin{eqnarray}\label{eq:subs}
\dfrac{\hbar}{2\pi}\int^{\infty}_{0}d\xi \longleftrightarrow k_{B}T{\sum^{\infty}_{l=0}}' ,
\end{eqnarray}

in \eqref{CasimirEnergy} together with the replacement of $\xi$ with $\xi_{l}= 2\pi\frac{k_{B}T}{\hbar}l$, the discrete Matsubara frequencies, takes into account the effect of temperature. We have defined $k_{B}$ to be Boltzmann's constant and the prime denotes that the term $l=0$ contains a prefactor $\frac{1}{2}$ compared to the other terms in the sum. This set of substitutions imply some assumptions which we now briefly discuss.\\
First of all we note that formally the dielectric function can also have temperature dependence through the parameters $\omega_{R_{i}}$,$\omega_{e_{i}}$ and $\gamma_{i}$  defined in \eqref{eq:phendiel}. Although to our knowledge there is no experimental data for topological insulators, these parameters are almost temperature independent for most dielectrics and so we exclude this effect in our analysis.
In addition, it is known that all dielectrics have non zero conductivity $\sigma(T)$ at $T \neq 0$ which modifies the dielectric function through $\epsilon(\omega, T) = \epsilon(\omega) + i4\pi\frac{\sigma(T)}{\omega}$. For dielectrics $\sigma(T)$ depends on the band gap $\Delta$: $\sigma(T)\sim \mathrm{exp}( -\frac{\Delta}{2k_{B}T})$.\\
Topological insulators such as Bi$_{2}$Se$_{3}$ have $\Delta \sim 0.3$eV \cite{XWQ09} and so we can neglect this contribution as a first approximation for temperatures below $T\sim 3\cdot10^{3}$ K which is enough for practical purposes. Nevertheless, it is possible to show \cite{BKMM09} that the inclusion of the finite conductivity term within the Lifshitz formalism leads to a violation of Nernst theorem which states that the entropy should tend to zero when $T\rightarrow 0$. Physically this is related to the appearance of a drift current, which leads to Joule heating and violates the condition of thermal equilibrium, necessary to apply the Lifshitz theory. Hence, the inclusion $\sigma(T)$ is therefore not justified within the Lifshitz theory and leads to large, unphysical thermal corrections which do not account for experimental data \cite{BKMM09}. Either way, we are forced to neglect this contribution. Other effects of temperature on the coating are discussed in section \ref{sec:conc}.\\
Having considered these points, we will assume that the formal substitution \eqref{eq:subs} is enough to take into account the effect of temperature on the Casimir effect in anisotropic topological insulators.

\subsection{Results at $T\neq0$ isotropic plates}

Once established the method to include temperature effects we analyze the case of two isotropic topological insulating plates described by (\ref{eq:phendiel}) at $T\neq0$. The Lifshitz equation (\ref{CasimirEnergy}) transforms for finite temperatures to:

\begin{equation}
\label{CasimirEnergytemp}
\frac{E_{c}(d)}{A} = k_{B}T{\sum^{\infty}_{l=0}}' \int \frac{d^2 {\bf k}_{\|}}{(2\pi)^2} \log \det \left[1 - {\bf R}_1 \cdot {\bf R}_2 e^{-2 k_3 d}\right].
\end{equation}

Where the transverse momentum $k_3$ is now evaluated at discrete frequencies $\xi_{l}$ such that $k_3=\sqrt{\bm{k}^{2}_{\|}+ \xi_{l}^2/c^2}$. It is convenient to define the adimensional temperature $\bar{T}$:

\begin{eqnarray}
\bar{T}\equiv \dfrac{2\pi k_{B}T}{\hbar\omega_{R}}.
\end{eqnarray}

For frequencies in the optical region, $\bar{T}=1$ correspond to temperatures $T\sim 2\cdot10^{3}$ K, while frequencies in the microwave region $\bar{T}=3.7$ correspond to temperatures $T\sim 300$K. Since we will be interested in the latter (the topological insulator TlBiSe$_{2}$ has a resonance frequency\cite{Chen10} at $\omega_{R}=56$cm$^{-1}$) our plots will range from $\bar{T}=0$ to $\bar{T}=10$. We note that the behavior is dominated by low frequency resonances as long as higher resonance frequencies have similar oscillator strengths in \eqref{eq:phendiel} (see auxiliary material in Ref.\cite{GC10}). Because of this, and the absence, to our knowledge, of broad frequency experimental data regarding the optical response of topological insulators (due mainly to their interest as thermoelectrics) we assume that this is the case and restrict to a one oscillator model throughout the paper. Nevertheless, as optical data becomes available, it is simple to implement these techniques and substitute the relevant parameters in the model since the overall assumptions will still hold (namely, the insulating behavior and the existence of a topological magnetoelectric polarizability).

We end here the discussion regarding the model and the theoretical tools and we now proceed to analyze both numerically and analytically the results obtained from integrating \eqref{CasimirEnergytemp}.

\subsubsection{Classical ($T\rightarrow\infty$) and quantum ($T\rightarrow 0$) limits}

To get some insight into the finite temperature behavior of the system one can ask what happens to the Casimir force in the (formal) limits when $T\rightarrow\infty$ and $T\rightarrow\ 0$. Trivially, if one first sets $T\rightarrow 0$ the expression (\ref{CasimirEnergy}) is recovered and the analysis of Ref. \cite{GC10} still holds. Hence a region of repulsion is expected to exist if the topological magnetoelectric polarizabilities of the plates have different signs.
For high temperature, $T\rightarrow\infty$ also referred to as the classical limit, all the terms in the $l$ sum above are exponentially suppressed except for the $l=0$ term \cite{BKMM09}. Thus, for isotropic plates, the dielectric function can be replaced by the zero frequency dielectric function. Let us derive the reflection coefficients in this case.\\
Directly from \eqref{eq:ReflectionMatricesTIcomplete}, and taking into account that $n^2_i=\epsilon_{i}$ the reflection coefficients at zero frequency take the form:

\begin{eqnarray}
r_s &=& \dfrac{1}{\Delta_{l=0}}(1-\epsilon(0)-\bar{\alpha}^2 +\sqrt{\epsilon(0)}\chi_{-}(0,\boldsymbol{k}_{\parallel})) \\
r_s &=& \dfrac{1}{\Delta_{l=0}}(-1+\epsilon(0)+\bar{\alpha}^2 +\sqrt{\epsilon(0)}\chi_{-}(0,\boldsymbol{k}_{\parallel})) \\
r_{sp} &=& \dfrac{2\bar{\alpha}}{\Delta_{l=0}} = r_{ps},
\end{eqnarray}

where $\Delta_{l=0} = 1+\epsilon(0)+\bar{\alpha}^2+\sqrt{\epsilon(0)}\chi_{+}(0,\boldsymbol{k}_{\parallel})$. From their definition \eqref{eq:Xipm}, the functions $\chi_{\pm}$ at zero frequency can be expressed in terms of $\epsilon(0)$ only ($\boldsymbol{k}_{\parallel}$ dependence cancels in this limit):

\begin{eqnarray}
\chi_{\pm} = \sqrt{\epsilon(0)}(1 \pm \dfrac{1}{\epsilon(0)})
\end{eqnarray}

Bringing together all simplifications the reflection coefficients (\ref{eq:ReflectionMatricesTIcomplete}) take the form:

\begin{eqnarray}
\label{eq:ReflectionMatricesTIinftemp}
{\bf R}_i = \dfrac{1}{2(\epsilon(0)+1)+\bar{\alpha}^2}\left(
\begin{array}{cc}
  -\bar{\alpha}^2  &  2 \bar{\alpha} \\
  2 \bar{\alpha} & 2(\epsilon(0)-1)+\bar{\alpha}^2
\end{array} \right),
\end{eqnarray}

We emphasize that although similar in structure, these reflection coefficients are different to the ones obtained at zero temperature and  $d \rightarrow \infty$ in appendix \ref{App:Minimum} by rescaling the Casimir energy density with $d$.\\
One can introduce this expression in \eqref{CasimirEnergytemp} and study the behavior of the Casimir energy as a function of the two parameters of the model: $\epsilon(0)=1+\frac{\omega^2_{e}}{\omega^2_{R}}$ and $\theta_{1,2}$. In this case one can rescale the integration variables with $d$ and focus on the force defined as $F=-\partial_{d}E_{c}(d)$ which takes the form:

\begin{equation}\label{eq:classicalforce}
F_{cl}(d) = \dfrac{k_{B}T}{d^3\pi}f(\epsilon(0),\theta_{1},\theta_{2}),
\end{equation}

where $f$ is a complicated integral expression of the parameters (see appendix \ref{App:class} for details). It is evident from the functional form of \eqref{eq:classicalforce} with $d$ that in the classical limit the Casimir force is either attractive or repulsive for all distances, depending only on the sign of $f$. Thus, in contrast to the zero temperature case, no equilibrium point is expected.\\
When $\mathrm{sgn}(\theta_{1})=\mathrm{sgn}(\theta_{2})$ no repulsion is obtained for any values of the parameters, as expected from the results in Ref.\cite{GC10}. Whenever $\mathrm{sgn}(\theta_{1}) \neq \mathrm{sgn}(\theta_{2})$ it is possible to draw the diagram of Fig. \ref{phasediagram} where the attractive and repulsive behaviors are shown as a function of the two parameters for the particular case where $\theta_{1}=-\theta_{2} \equiv\theta$. To understand this diagram one first has to note that the topological magnetoelectric polarizability has an upper bound to satisfy the positive energy condition\cite{BHS68} for magnetoelectric materials. In the present context, this condition implies that $\frac{\alpha|\theta|}{\pi} < \sqrt{\epsilon(0)}$ which excludes the black region on the right of Fig. \ref{phasediagram}. The other two regions indicate attractive (white top region) or repulsive (green low region) behavior. From this diagram it is transparent that even in the classical limit of very high temperature there exists a region of parameters where complete repulsion is obtained. It is relevant to point out that a low dielectric response is needed for this to happen. High topological magnetoelectric polarizability also enhances the repulsive behavior.\\
\begin{figure}
\includegraphics[scale=0.9]{Fig3}
\caption{\label{phasediagram}(color online) Attraction versus repulsion in the classical limit ($T\rightarrow\infty$) as a function of $\frac{\omega_{e}}{\omega_{R}}$ and $\frac{\theta}{\pi}$ where $\theta_{1}=-\theta_{2} \equiv\theta$. The white upper region shows attraction while the lower green region shows repulsion. The black region is a forbidden region for the parameters due to the positive energy condition $\frac{\alpha|\theta|}{\pi} < \sqrt{\epsilon(0)}$ (see text).}
\end{figure}
Can one understand the origin of repulsion in the classical limit analytically? The answer is in fact affirmative. For small $\theta_{1,2}$ and $1-\epsilon(0)$, it is possible to write a closed analytical form for the Casimir force of the parameters although for the sake of clarity we leave this to appendix \ref{App:class}. In addition to this, we have included a discussion of the classical limit in terms of the Casimir energy density (see appendix \ref{App:class}) in the spirit of reference \cite{GC10} studying the relative strength of the diagonal and off-diagonal reflection coefficients. Both approaches lead to the same result: repulsion is possible in the classical limit for a certain range of parameters which are summarized in Fig.\ref{phasediagram}. Having studied these limiting cases we know proceed to the general case where $T\neq 0$.

\subsubsection{$T\neq 0$: the general case}

The effect of increasing temperature for a situation where $\mathrm{sgn}(\theta_{1})=-\mathrm{sgn}(\theta_{2})$ is presented in Fig.\ref{Fig:finiteT}. In general, temperature acts against repulsive behavior, driving it towards shorter distances as temperature increases. The evolution of the equilibrium position with respect to the adimensional temperature $\bar{T}$ is shown in Fig. \ref{Fig:finiteT}(b). For high values of $\bar{T}$ ($\bar{T}>5$) it is possible to complete equation \eqref{deqproptheta} (valid for small values of $\theta_{1,2}$) to write:

\begin{eqnarray}\label{deqpropthetaT}
\bar{d}_{eq}\propto  \dfrac{|\theta_{1}\theta_{2}|}{\bar{T}}.
\end{eqnarray}

\begin{figure*}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.39]{Fig4a}
(a)
\end{minipage}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.40]{Fig4b}
(b)
\end{minipage}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.40]{Fig4c}
(c)
\end{minipage}
\caption{\label{Fig:finiteT}(color online) (a) Casimir energy density (in units of $E_{0}= A\hbar c/(2\pi)^2(\omega_{R}/c)^3$) as a function of the dimensionless distance $\bar{d}$ for $\frac{\omega_{e}}{\omega_{R}}=0.45$ for temperatures ranging from $\bar{T}= 0-10$ and $\theta_{1}=-\theta_{2} = 3\pi$. Temperature pushes the repulsive behavior to shorter distances. (b) Equilibrium distance as a function of temperature. (c) Casimir energy density (in units of $E_{0}= A\hbar c/(2\pi)^2(\omega_{R}/c)^3$) as a function of $\bar{d}$ for $\frac{\omega_{e}}{\omega_{R}}=0.16$ for temperatures ranging from $\bar{T}= 0-10$. For values where there is repulsion, decreasing the temperature shifts the curve towards smaller distances as shown inside the inset figure.}
\end{figure*}

This simple relation, extracted from numerical data, shows that for small topological magnetoelectric charge and high temperature both effects compete as regards to the equilibrium position.\\
One can summarize the results for this section as follows. In the classical limit, one can have either attraction or repulsion, regardless of the distance. Starting with attraction at the classical limit, i.e $\bar{T} \rightarrow \infty$, decreasing temperature will develop a deeper minimum which will shift to longer distances as shown in Fig.\ref{Fig:finiteT}(a) and (b). Consistent with the discussion presented the end of section \ref{sec:T=0}.B, in some special cases where the magnetoelectric is bigger than a critical value one can end with repulsion at $T=0$ without a minimum.\\
Starting from repulsion in the classical limit will not develop a minimum when decreasing $\bar{T}$ but it will shift the curve of repulsive behavior towards larger distances to end with repulsion in the quantum limit. This is shown in Fig.\ref{Fig:finiteT}(c). It must be noted that for this to happen, a very low $\epsilon(0)$ is needed when $\theta\sim\pi$ and as $\theta$ is increased, higher $\epsilon(0)$ are capable of giving rise to the complete repulsive behavior. Therefore we expect this not to be the relevant situation for real topological insulators, which have low $\theta$, but rather the one presented in Fig. \ref{Fig:finiteT}(a). An extension of this analysis could be relevant for other magnetoelectric materials such as Cr$_{2}$O$_{3}$ that can present higher axion coupling as well as more general magnetoelectric couplings \cite{Obu08}.\\
We note for completeness that when both topological magnetoelectric couplings have equal signs, temperature acts to increase attraction as expected from ordinary dielectrics.\\
We finish this section with a technical comment regarding the commutativity of the limits. We have discussed the high and low temperature limits, and studied the distance dependence numerically. At this point, one might ask whether the limits commute, i.e. if one evaluates first the  $d\rightarrow 0$ or $d\rightarrow \infty$ limit first and then consider $T\rightarrow 0$ and $T\rightarrow \infty$, would the result remain as stated above?
The fact is that in some cases, the limits commute while in others they do not. In particular, is clear from expression \eqref{CasimirEnergytemp} that the limits $d\rightarrow \infty$ and $T\rightarrow \infty$ will commute. It is easy to show that, in either order, both result into the same reflection coefficients given by \eqref{eq:ReflectionMatricesTIinftemp}. For the case when $d\rightarrow 0$ and $T\rightarrow 0$ a similar situation occurs and the limits also commute. The interesting case is however when $d\rightarrow 0$ and $T\rightarrow \infty$ (or viceversa). If one expands the exponential function, then taking the temperature to infinity breaks down the expansion and this limit is not reconciled with the $T\rightarrow \infty$, $d\rightarrow 0$ which typically gives attraction. Although it might seem surprising at first, one should recall other physical situations where a similar situation happens, one particularly impressive example taking place when calculating the DC or minimal conductivity of graphene where the order of evaluating the limits is crucial (for a recent review of the problem see Ref.\cite{SAHR10} section IV.A). Nevertheless, it should be noted that, with the numerical results in mind, there is a way around the puzzle by imposing that we take the limits in such a way that the product $Td$ is a constant. In this way, the $l=0$ is the leading term in the sum \eqref{CasimirEnergytemp} and we recover the reflection coefficients \eqref{eq:ReflectionMatricesTIinftemp} relevant for high temperature, making the limits commute.

\section{\label{sec:uniaxial}Casimir force between topological insulators with uniaxial anisotropy at $T=0$}

In this section we again set the temperature to zero and focus on the effect that uniaxial anisotropy has on the repulsive behavior.

\subsection{Anisotropy in topological insulators}

For a given material its linear response to an electromagnetic wave, or in turn, its reflection coefficients defined in (\ref{CasimirEnergy}) depend strongly on the dielectric tensor $\epsilon_{ij}$, the magnetic susceptibility tensor $\mu_{ij}$ and the magnetoelectric tensor $\theta_{ij}$. Since we are dealing with non magnetic topological insulators we will assume that $\mu_{ij}=\delta_{ij}$, although we shall derive the reflection coefficients for the general case in which the susceptibility is considered.

Crystal symmetry defines the other two tensors. Due to time reversal symmetry, for topological insulators the magnetoelectric tensor can only have the form $\theta_{ij}=\theta\delta_{ij}$ with $\theta=\pi$  (mod($2\pi$)) for topological insulators and $\theta =0$ for ordinary insulators \cite{EJV10}. It is interesting to note that for general magnetoelectric crystals, other magnetoelectric couplings can be present in the action \eqref{eq:lagrangean}, and $\theta_{ij}$ could have a more elaborate form \cite{LL8, EJV10} which could in principle affect the sign of the Casimir force. We will restrict ourselves to the case of a constant isotropic magnetoelectric tensor $\theta_{ij}=\theta\delta_{ij}$, relevant for crystalline topological insulators \cite{EJV10}.\\
The form of $\epsilon_{ij}$ is also determined by crystal symmetry and one can distinguish the cubic, uniaxial and biaxial crystals\cite{LL8}. The simplest case, the cubic structure, has $\epsilon_{ij}=\epsilon(\omega)\delta_{ij}$, which is just the isotropic case considered in previous sections. Although interesting as a first approximation \cite{GC10}, this model is incomplete for topological insulators. The prototypical examples of topological insulating crystals Bi$_2$Se$_3$, Bi$_2$Te$_3$ , Sb$_2$Te$_3$ \cite{Chen10,C09,X09} or the novel Thallium based III-V-VI$_{2}$ compounds \cite{Zhang10,Chen10,LMW10a,LMW10b} have rhombohedral symmetry, which fall into the category of uniaxial crystals and hence we will focus on this case, leaving biaxial crystals aside. Uniaxial crystals have a definite optical axis which coincides with the principal crystal axis. The dielectric tensor can thus be written in the form: $\epsilon_{ij}=\mathrm{diag}(\epsilon_{\perp},\epsilon_{\perp},\epsilon_{z})$, where the optical axis is aligned with the $z$ axis. In all our calculations, the optical axis of the two Casimir plates are supposed to be aligned so that no torque is induced in the system \cite{BKMM09}.

\subsection{Fresnel coefficients for topological insulators with uniaxial anisotropy at $T=0$}

Fresnel coefficients are derived from Maxwell's equations by imposing continuity relations for the normal components of $\bf{D}$ and tangential components of $\bf{H}$ as discussed above for the isotropic case (see appendix \ref{App:coef}). After some tedious but straightforward work one obtains the reflection matrices for an anisotropic topological insulator-vacuum interface:

\begin{widetext}
\begin{eqnarray}
\label{eq:anisotropicandTI}
\mathbf{R}_{i} =\dfrac{1}{\Delta_{an}}\left(
\begin{array}{cc}
\left(\mu_{\perp}k_{z}-q'\right) \left(\epsilon_{\perp}k_{z}+q'' \right)-q''k_{z}\mu_{\perp}\bar{\alpha}^2  & 2\bar{\alpha}q''\mu_{\perp}k_{z}\\
  2\bar{\alpha}q''\mu_{\perp}k_{z} & \left( \epsilon_{\perp}k_{z}-q''\right) \left(\mu_{\perp}k_{z}+q' \right)+q''k_{z}\mu_{\perp}\bar{\alpha}^2
\end{array} \right),
\end{eqnarray}
\end{widetext}

where $\Delta_{an}= \left( \mu_{\perp}k_{z}+q'\right) \left(\epsilon_{\perp}k_{z}+q'' \right)+q''k_{z}\mu_{\perp}\bar{\alpha}^2 $, $k^2_{z} = \dfrac{\omega^2}{c^2}-k^{2}_{\parallel}$, $q'^{2} = \dfrac{\omega^2}{c^2}\epsilon_{\perp}\mu_{\perp}-k^2_{\parallel}\dfrac{\mu_{\perp}}{\mu_{z}}$, $q''^{2} = \dfrac{\omega^2}{c^2}\epsilon_{\perp}\mu_{\perp}-k^2_{\parallel}\dfrac{\epsilon_{\perp}}{\epsilon_{z}}$ and $\bar{\alpha} = \alpha\theta/\pi$.
To compute the Casimir energy, one should define these in the imaginary frequency axis and perform the substitution $\omega = i\xi$.
We stress that these reduce to the ordinary anisotropic coefficients presented in appendix \ref{App:coef} when $\bar{\alpha}=0$. They also reduce to the isotropic reflection coefficients \eqref{eq:ReflectionMatricesTIcomplete} when $\mu$ and $\epsilon$ are isotropic.\\
To investigate the effect of anisotropy it is necessary to model the dielectric response of the material. In general, insulators can be described by its resonance frequencies, hence we model $\epsilon_{\perp}$ and $\epsilon_{z}$ with a sum of oscillators:

\begin{eqnarray}\label{eq:phendiel1}
\epsilon_{z}(i\xi) &=& 1+\sum_{i}\dfrac{\omega_{e_{z},i}^2}{\xi^2+\omega^2_{R_{z,i}}+\gamma_{z,i}\xi}, \\
\label{eq:phendiel2}
\epsilon_{\perp}(i\xi) &=& 1+\sum_{i}\dfrac{\omega_{e_{\perp},i}^2}{\xi^2+\omega^2_{R_{\perp,i}}+\gamma_{\perp,i}\xi}.
\end{eqnarray}

We have evaluated the dielectric function at imaginary frequencies, as demanded by equation \eqref{CasimirEnergy}. The parameters $\omega_{e_{\perp,i}}$ and $\omega_{e_{z,i}}$ indicate the strength of the oscillator while $\omega_{R_{\perp,i}}$ and $\omega_{R_{z,i}}$ account for the resonance frequencies of the oscillators. Finally, we include the damping parameters $\gamma_{\perp,i}$ and $\gamma_{z,i}$ for completeness although they do not play a mayor role on Casimir physics.

A multiple oscillator model does not significantly alter the general behavior of the Casimir force\cite{GC10} and so, in order to clarify the effects that different parameters have on the Casimir energy density we will restrict the models \eqref{eq:phendiel1} and \eqref{eq:phendiel2} to one oscillator models. In this scheme we will investigate two aspects: (i) the effect of modifying the relative strength of the parallel component against the perpendicular i.e. $\omega_{e_{z}}$ over $\omega_{e_{\perp}}$ and (ii) the effect of the relative movement of the position of the resonance frequencies $\omega_{R_{\perp}}$ and $\omega_{R_{z}}$.

\subsection{Effect of the relative strength of the parallel component against the perpendicular component}

To study this effect we simplify equations \eqref{eq:phendiel1} and \eqref{eq:phendiel2} to unmask the effect under study (i.e. point (i) above). Redefining the parameters in units of $\omega_{R_{\perp}}$:

\begin{eqnarray}\label{eq:phendiel1p1}
\epsilon_{z}(i\xi) &=& 1+\dfrac{\omega_{e_{z}}^2}{\xi^2+ 1 +\gamma\xi}, \\
\label{eq:phendiel2p1}
\epsilon_{\perp}(i\xi) &=& 1+\dfrac{\omega_{e_{\perp}}^2}{\xi^2+ 1 +\gamma\xi}.
\end{eqnarray}

In this case we have chosen $\omega_{R_{\perp}}=\omega_{R_{z}}$ and $\gamma\equiv\gamma_{R_{\perp}}=\gamma_{R_{z}}=0.01$ in units of $\omega_{R_{\perp}}$ . To study the effect of changing the relative strength of the dielectric components we may fix $\omega_{e_{z}}=0.45$ (in units of $\omega_{R_{\perp}}$) and change $\omega_{e_{\perp}}$ in the interval $0-1$. The results are shown in Fig.\ref{Fig1}. We have fixed $\theta_{1}=-\theta_{2}=0$ (i.e. the topologically trivial anisotropic case) in Fig. \ref{Fig1}(a), $\theta_{1}=\theta_{2}=\pi$ in Figure \ref{Fig1}(b) and $\theta_{1}=-\theta_{2}=\pi$ in Fig. \ref{Fig1}(c).

\begin{figure*}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.39]{Fig5a}
(a)
\end{minipage}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.4]{Fig5b}
(b)
\end{minipage}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.4]{Fig5c}
(c)
\end{minipage}
\caption{\label{Fig1} (color online)Effect of changing the relative oscillator strengths between parallel and perpendicular components of the dielectric function on the Casimir energy density (in units of $E_{0}= A\hbar c/(2\pi)^2(\omega_{R_{z}}/c)^3$) as a function of the dimensionless distance $\bar{d}$ with (a) $\theta_{1,2}=0$ and (b) $\theta_{1}=\theta_{2}=\pi$ (c) $\theta_{1}=-\theta_{2}=\pi$. (a) Attraction is obtained as no magnetoelectric term is included. (b) Both magnetoelectric couplings have the same sign and so no repulsion occurs. (c) Repulsion appears at short distances. Increasing $\omega_{e_{\perp}}$ makes the minimum shift to lower distances while increasing its depth. Therefore, repulsion is favored by the condition $\omega_{e_{z}}>\omega_{e_{\perp}}$ }
\end{figure*}

Fig. \ref{Fig1}(a) is a reference figure where only anisotropy is studied with $\theta=0$. In this case, attraction occurs since $\theta_{i}=0$ and there is no mixing of polarizations since the diagonal component in \eqref{eq:anisotropicandTI} is zero (see appendix \ref{App:coef}). As $\omega_{e_{\perp}}$ grows the tendency is to favor attraction and to increase the absolute value of the Casimir energy at a given distance. In Fig. \ref{Fig1}(b) the magnetoelectric terms have equal sign and so no repulsion is obtained just as it is expected from the isotropic case\cite{GC10}. When $\theta_{1}$ and $\theta_{2}$ have opposite sing, $\theta_{1}=-\theta_{2}=\pi$, the Casimir energy develops a minimum, shown in Fig. \ref{Fig1}(c). The actual distance at which the minimum appears is shifted to shorter distances as $\omega_{e_{\perp}}$ is increased. This enables to draw the conclusion that for the minimum to shift to larger distances, or in other words, for the repulsive behavior to be enhanced, the material in question has to favor the strength of oscillators in the direction parallel to the optical axis. \\
Physically, repulsion in this system is due to the mixing of polarizations\cite{GC10}. Thus, suppression of repulsion can be traced back to the relative suppression of the off-diagonal terms in \eqref{eq:anisotropicandTI} versus the diagonal terms just as in the anisotropic case studied in \cite{GC10}. When increasing $\epsilon_{\perp}$ fixing $\epsilon_{z}$ to a constant, the off-diagonal terms vanish, confirming the numerical analysis.

\subsection{Effect of the relative position of the oscillator frequencies}

To study this case, the dielectric functions of both components can be written as:

\begin{eqnarray}\label{eq:phendiel1p2}
\epsilon_{z}(i\xi) &=& 1+\dfrac{\omega_{e}^2}{\xi^2+ 1 +\gamma\xi}, \\
\label{eq:phendiel2p2}
\epsilon_{\perp}(i\xi) &=& 1+\dfrac{\omega_{e}^2}{\xi^2+ \beta +\gamma\xi}.
\end{eqnarray}

In this case we have chosen $\omega_{e_{\perp}}=\omega_{e_{z}}\equiv \omega_{e}=0.45$ and as before  $\gamma=0.01$ (in units of $\omega_{R_{\perp}}$). The parameter $\beta\equiv \frac{\omega^2_{R_{\perp}}}{\omega^2_{R_{z}}}$ determines the relative position between both oscillators: for $\beta>1$, $\epsilon_{\perp}$ has a higher resonance frequency than $\epsilon_{z}$ and for $\beta<1$ the opposite situation occurs. Again we have fixed $\theta_{1}=-\theta_{2}=0$ in Fig. \ref{Fig2}(a), $\theta_{1}=\theta_{2}\equiv\theta_{b}=\pi$ in Fig. \ref{Fig2}(b) and $\theta_{1}=-\theta_{2}\equiv\theta_{c}=\pi$ in Fig. \ref{Fig2}(c).

\begin{figure*}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.39]{Fig6a}
(a)
\end{minipage}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.4]{Fig6b}
(b)
\end{minipage}
\begin{minipage}{.32\linewidth}
\includegraphics[scale=0.4]{Fig6c}
(c)
\end{minipage}
\caption{\label{Fig2}(color online) Effect of changing the relative positions of the oscillator resonances between parallel and perpendicular components of the dielectric function on the Casimir energy density (in units of $E_{0}= A\hbar c/(2\pi)^2(\omega_{R_{z}}/c)^3$) as a function of the dimensionless distance $\bar{d}$ with (a) $\theta_{1,2}=0$ and (b) $\theta_{1}=\theta_{2}=\pi$ (c) $\theta_{1}=-\theta_{2}=\pi$. (a) Attraction is obtained as no magnetoelectric term is included. (b) Both magnetoelectric couplings have the same sign and so no repulsion occurs. (c) Increasing $\omega_{R_{\perp}}$ makes the minimum shift to higher distances while decreasing its depth. Therefore, repulsion is favored by increasing $\beta$.(see text)}
\end{figure*}

As in the previous case, Fig. \ref{Fig2}(a) a reference figure where only parameter $\beta$ is modified. We have chosen the values of $\beta$ ranging from $\beta=10^{-3}$ to $\beta=10^{3}$, so a broad range of situations are represented. In this situation, attraction occurs since $\theta_{i}=0$ and there is no mixing of polarizations. As $\beta$ grows the tendency is to favor attraction and to increase the absolute value of the Casimir energy at a given distance. In Fig. \ref{Fig2}(b) the magnetoelectric terms have equal sign and so no repulsion is obtained. Fig. \ref{Fig2}(c) shows how the minimum is shifted to lower distances as $\omega_{R_{\perp}}$ is increased, i.e. $\beta$ is increased. Hence, for the repulsive behavior to be favored, the material in question has to favor low resonance frequencies in the parallel direction, while high frequencies in the perpendicular direction. This is consistent with the behavior discussed above where suppression of $\epsilon_{\perp}$ enhances repulsion. In this case, increasing $\beta$ suppresses $\epsilon_{\perp}$ and favors repulsion \footnote{This effect is analogous to the effect discussed in Ref. \cite{GC10} (auxiliary information) where a higher oscillator frequency was studied and seen to enhance repulsion.\\}. \\
We summarize the results of this section in what follows. From the numerical results one can readily infer what conditions are necessary for repulsion to be observed, given that the topological magnetoelectric terms of the two materials have opposing signs. For the repulsive behavior to appear at the largest distances possible, one should search for a material where the direction parallel to the optical axis has a bigger oscillator strength than the corresponding strength of the oscillator in the parallel direction $\omega_{e_{z}}>\omega_{e_{\perp}}$. Further enhancement of the repulsive behavior can be achieved if the oscillator resonances in the direction perpendicular to the optical axis are at higher frequency than resonances for the parallel direction, i.e $\omega_{R_{z}}>\omega_{R_{\perp}}$. In both situations, $\epsilon_{\perp}$ is suppressed relative to $\epsilon_{z}$ and the mixing of polarizations is maximized.\\
With these numerical calculations we have established the main directions to enhance repulsive behavior with topological insulators at low temperature. We now discuss the effect of temperature on these findings.

\section{\label{sec:uniaxialandtemp}Casimir force between topological insulators with uniaxial anisotropy at $T\neq0$}

The result of including the two effects subject of this work, temperature and anisotropy together is shown in Fig \ref{Fig:Anistemp}. To illustrate that the repulsive behavior is still present we study two different cases. In the first of them, corresponding to Fig. \ref{Fig:Anistemp}(a) we vary the adimensional temperature from $\bar{T}=0$ to $\bar{T}=7$ while fixing the uniaxial anisotropy parameters and $\theta_{1}=-\theta_{2}=\pi$. In particular we fix the oscillators strengths to $\omega_{e_{z}}=0.45$, $\omega_{e_{\perp}}=0.3$ and the relative position of the resonances to $\beta=5$, i.e. the perpendicular oscillator is shifted by a factor of five with respect to $\omega_{R_{z}}$. As expected by previous sections, the figure proves that temperature works against the repulsive behavior, shifting repulsion to shorter distances as temperature is increased. In a second situation we illustrate the effect of varying anisotropy at a given temperature. In this case, we fix the temperature to $\bar{T}=5$, the oscillator strength in the parallel direction to $\omega_{e_z}=0.45$ and $\beta=5$ while varying $\omega_{e_{\perp}}$ from $\omega_{e_{\perp}}=0$ to $\omega_{e_\perp}=1$. The results show that enhancing perpendicular response, even at finite temperature, favors repulsive behavior. Consistently with previous sections, equal signs of $\theta_{1,2}$ the system returns to attraction at all distances.

\begin{figure*}
\begin{minipage}{.49\linewidth}
\includegraphics[scale=0.5]{Fig7a}
(a)
\end{minipage}
\begin{minipage}{.49\linewidth}
\includegraphics[scale=0.5]{Fig7b}
(b)
\end{minipage}
\caption{\label{Fig:Anistemp}(color online) Casimir energy density (in units of $E_{0}= A\hbar c/(2\pi)^2(\omega_{R,z}/c)^3$) and $\theta_{1}=-\theta_{2}=\pi$ including anisotropy and temperature effects: (a) Effect of changing the temperature from $\bar{T}=0 - 7$ with $\omega_{e,z}=0.45$, $\omega_{e,\perp}=0.3$ and $\beta=5$. (b) Effect of varying $\omega_{e,\perp}=0-1$ with $\bar{T}=5$, $\omega_{e,z}=0.45$ and $\beta=5$.}
\end{figure*}

\section{\label{sec:conc}Discussion and Conclusions}

In this work we have studied the effect of anisotropy and temperature on the repulsive Casimir effect with three dimensional topological insulators. We have found that the repulsive behavior is still present even when including these effects. In particular, increasing temperature tends to reduce repulsion, similar to what is expected from different situations such as metamaterials \cite{Rosa08}. On the other hand, enhancing the optical response in the direction parallel to the optical axis of the topological insulator works in favor of repulsion. This can be achieved either by increasing the relative strength of the oscillator in the parallel direction or by searching for resonance frequencies which suppress the perpendicular response. We have also determined that both effects together still allow for repulsion. All these effects can be understood as an enhancement of the off-diagonal terms in the reflection coefficients, which favors polarization mixing and thus repulsion, whenever the signs of the topological magnetoelectric terms are opposite in both plates.  \\
Although these specific conclusions are reached, it is difficult to draw conclusions for real materials since the optical response of topological insulators still needs further experimental characterization. In particular, values for the optical parameters are still lacking, in contrast with other materials which are traditionally useful for measuring the Casimir force \cite{BKMM09,Palik98}. Nevertheless, in this work, we have aimed also to establish the theoretical framework for handling anisotropy in topological insulators in the context of their optical properties, which to our knowledge was absent in the literature. The reflection coefficients for anisotropic materials can also be helpful in achieving the optical characterization of these materials and could be relevant for metrology purposes, as suggested in previous works\cite{TM10,MQDZ10}. This theoretical work on anisotropy might also be used as a starting point for the study of the Casimir force in situations involving other magnetoelectric materials.\\
A final issue left out in this work is the effect of temperature on the magnetic coating. Even though magnetic interactions where shown to be irrelevant \cite{GC10}, temperature will have an effect on the magnetization. In particular, the magnetic moments will fluctuate with increasing temperature and destroy ferromagnetism when the system is over the Curie temperature ($T_{c}$) of the coating. This temperature depends on the specific coating material which should be an insulating or semiconducting ferromagnet with as high as possible Curie temperature.
Although ferromagnets are usually metallic, examples of insulating ferromagnets exist, for example oxides such as the rare earth oxide $Eu0$ with Curie temperature close to $70$K \cite{H78}, and have been synthesized and used in the past, such as the ferromagnetic insulator GdN. The latter has been shown to have a Curie temperature close to $60$K \cite{H78}, it can be grown as a thin film of thickness $\sim6$nm\cite{XC96} and could be a suitable candidate for the ferromagnetic covering. \\
In conclusion we expect that the tools and behaviors studied in this work might lead towards a complete optical characterization of topological insulators, a first step towards Casimir like experiments in which the description of factors such as temperature and anisotropy should be relevant.

\section*{Acknowledgements}

Two of us, A.G.G. and A.C., are indebted to M.A.H. Vozmediano for fruitful conversations and encouraging discussions. A.G.G. has enjoyed conversations with T. Emig and acknowledges financial support from MICINN through grant No. FIS2008-00124 (FPI Program). P.R.-L. acknowledges helpful discussions with R. Brito. P.R.-L. research supported by projects MODELICO, MOSAICO and a FPU MEC grant. A.C. acknowledges Alianza 4 Universidades Program for funding.

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When is an ECSI document used?
It is good practice, in international trade, to almost always create an Export Cargo Shipping Instruction, or at least complete one as part of your export documentation suite, so that you can clearly instruct the logistics provider on how to handle your goods in transit from you to your customer.
The document will also instruct the provider as to how the transport documents should be distributed and the name of the party responsible for the respective carriage charges Normally, the logistics company can generate an ECSI on your behalf. However, the goods are yours and you know best how they should be treated during transit, so it's advisable that YOU understand and complete the ECSI document yourself.
You can complete an ECSI by manually getting a paper ECSI and completing the relevant sections by hand. This approach is ideal if you only have to do an ECSI once or twice a year. Anything more often than that you would be better in investing with an online tool, like EdgeCTP, which guides you, step-by-step, field-by-field through the entire completion of the ECSI. The added benefits of doing the ECSI online is that any details you type in can be reused the next time, and completed with just a few clicks – saving you time and money.
The explanation steps below were completed using the EdgeCTP's ECSI online application and the focus is on the key and mandatory data items from an exporters point-of-view.
Add your business details to the Exporter/ Shipper section and any Customs (HMRC) references to assist with Customs declarations; the Booking Number is the logistics carrier reference associated with the export leg.
Add the buyer of importers name and address details.
Optionally, add the Freight Forwarder name and address details, who is responsible for consigning the shipment.
Optionally, if there is another party or address involved, then add their details here.
Optionally, if required complete the relevant two sections with the specified information.
Optionally, indicate any insurance details associated with the export consignment.
Indicate what documentation is required and who should be charged or produce the documentation (A, B, C, D or E).
Indicate what freight services are required and who should be charged for each service (A, B, C, D or E).
Optionally, provide any special instructions for stowing or transporting the consignment.
If the consignment is being shipped to a European Community member state (country) under Customs Controls, then specify the relevant status e.g. 'T1' otherwise leave this field blank.
Optionally, enter the name of the Port where the freight is payable, or leave empty if not applicable or state "pre-paid" if already paid or "destination" if payable at destination.
If required, enter the number of original and copies of Bills of Lading to be produced.
As the exporter, enter your: Company Name; Contact Telephone Number; Your Full Name and Position within your company; Place of Issue, where you're signing this declaration; Date of Issue, when you're signing this declaration and finally your Signature to complete the declaration.
Where can I get an ECSI document?
You can get your logistics firm or freight forwarder to provide you with a blank paper document of their Export Cargo Shipping Instruction form. Just make sure it's the UN or SITPRO aligned format.
Alternatively, if you'd like a digital ECSI, check out online platforms like EdgeCTP, which will give you an ECSI template onto which you can type, save and print your own data. It's not complicated and takes about 60 seconds to sign-up here for EdgeCTP on a free, no obligations, 30-days free trial basis, which means you can try this out risk-free.
If you do use EdgeCTP, then after signing-up and login into EdgeCTP, just go to the Documents tab and choose ECSI. The system will then allow you to type your data onto the face of the ECSI and generate a printable version.


Bibliographic coding in the first issue of "The New Age"
Bibliographic coding, according to George Borstein, is connected to Walter Benjamin's concept of "aura." He uses it to mean distinguishing features of a work (page layout, typeface, etc) that emphasize the work's "presence in time and space." In the first issue of "The New Age," the reader is struck by its similarity in appearance to a newspaper: black sarif font on white paper, with headlines in larger, bold print. There is no cover, per se. The front page includes the title of the publication, the date, its cost, and on the upper right and left corners, placed around the title that calls itself "an independent socialist review of politics, literature and art," we find small boxed advertisements - one for coffee, another for bread.
There is no table of contents; rather, the first two pages consist of a lengthy article addressing politics, wherein the sections are headlined with subheadings in bold capital letters (one assumes these are written by one or both of the editors, as there is no signature). On the third page, we find letters to the editor (again reminiscent of this type of section in a newspaper). Throughout this issue, scattered among the poetry, reviews, and essays, we find advertisements for lectures, books, and food.
The nature of what is advertised seems to underscore the socialist angle of the magazine - everyday food staples along with intellectual writings and lectures, the simple needs of an everyday socialist. Furthermore, the likeness of the magazine to a newspaper adds a perception of authority to what is said within its pages. The first two pages basically lay out an analysis of the current political situation in Britain, providing a framework through which the reader can then view the contents following it. The impression of authority given by its layout makes the reader less inclined to question the merits of what is being said within, and more inclined to allow the editors and authors published in "The New Age" to set the terms of the debate.
Read more about Bibliographic coding in the first issue of "The New Age"
The Bornstein reading discusses different theories of construction in a literary context. Not only is there a linguistic code which focusses on the words and content of the pieces, but there is also a bibliographic code. Bibliographic code refers to how the content is presented to the reader. Borstein describes that this could be spacing, cover design, or page layout. It affects how the words are delivered the reader and how they are interpreted. For example, if a piece is spaced in a certain way, that affects how it is read. The spaces can cause the reader to pause in certain places and that puts emphasis on certain words and phrases. Page layout can also affect how literature is processed by an audience. If it is designed in a certain way the eye may jump across the page in different patterns of visual flow charts.
For example on page 10 in issue No. 1 of "Blast," there is a different font used down the page. This emphasizes the words in different ways. Having the words capitalized or bolded makes certain phrases stand out compared to others. For example, the word automobilism is bolded and capitalized. This draws extra attention to it and makes what follows after it comparable to a definition.
I've chosen to look at the first issue of BLAST and just by looking at the cover, I've realized how different the bibliographic coding for the journal is looking at it on the web is versus having the copy that was scanned to produce this digital copy. The front cover and the back cover are two entirely different shades of pink. The front is very faded, and it almost looks like it started out a red-brown color. Compared to the bright and shocking pink of the back cover, I would never have guessed that the two started out the same exact color. It makes me wonder what exactly happened to the front cover, and perhaps having the physical copy for bibliographic coding would lend me more of an idea. It almost looks as though something spilled on the front cover. The binding is held together by what looks like old masking tape and both covers have rips and the pages are curled under. In the sense of experiencing the wear and age of the document, I scarcely connect with it through the digital version whereas I think I'd get a strong sense of it if I had the actual physical copy in my hands.
Delving into the text, I notice that the printing of the letters and images in the issue appears to be inexact. For example, there are spots where there are extra dots of black on the page, like on a page towards the beginning where it says MANIFESTO. and there is an image of what looks like a jousting weapon. Around the image, there are imperfections in the printing which I only noticed because I looked carefully for them and zoomed into the document from its default view on my computer. Likewise, scrolling two pages down to the page that begins BLAST First (from politeness) ENGLAND, I notice that just by looking at the letters A on the page and comparing them to one another, some of them have the triangle part on the top filled in while others are open to reveal white paper. There are also some spots in the black letters where white dots show, revealing more imperfections in the printing. This bibliographic coding is difficult to obtain and understand in the digitized versions. Had I not been looking closely, I would not have noticed it. Browsing through digitized versions is a very different experience from looking at a physical copy of something. It certainly changes the bibliographic coding as Borenstein mentioned when comparing King Lear originals to reprints. I wasn't so convinced that the experience would be very different from looking at a scanned version of BLAST and a physical copy, but now that I've examined it closer, I've come to a different conclusion. I'm sure this will be further evident after visiting the special collections to see a copy in person.
I couldn't help but notice the initial visual experience that exists, even in an archived copy, of the first issue of BLAST. Lewis's obsession with pure, abstract energy is evident in his own vorticist artwork, the typeface of "Manifesto--I," and the cover design itself, whose offset block-letter "BLAST" screams off the hot-pink backdrop that seems to glow from its own radiating energy.
However, much of Lewis' energy seems lost after the excitement of the first issue, both in content and the somber subject of the War itself. In his editorial, Lewis recognizes the effect of the war on Europe, but insists that "art should be fresher for the period of restraint." And although this issue has most of the same contributors, the lack of physical content alone shows their exasperated inability to keep up with the previous issue (with the exception of Lewis, who contributes a greater portion) but also in the more traditional typeface, and especially in the cover. Gaudier-Brzeska says it best in his "Vortex": "IT WOULD BE FOLLY TO SEEK ARTISTIC EMOTIONS AMID THESE LITTLE WORKS OF OURS." The drama in Europe, as this issue's contrast to the last shows, is not playing out on the artistic stage, but on the battlefield. As a result, BLAST's second issue cannot mimic the energy of the first, but instead adapts the aura of the era.
Thought some of you might like this article in the Times on Indian artist Nandalal Bose (1882-1966).
I just want to say that yesterday's presentations did a good job of bringing out the conflicts and contradictions in your respective aspects of The New Age. There was some good analysis as well as the exposure of some potentially fruitful points of research. For Monday, we'll hear from the two groups that still need to present and will then discuss Ardis, Morrisson and Bornstein. This will wrap up our study of The New Age and bring us into the wider world of avant-garde magazines and cultures. Our reading for Thursday 7/17 will consist solely of what you bring to the table in your readings of the other magazines at the MJP.
You'll also notice that I've changed the Descriptive Bibliography assignment to remove the presentations and place a focus on what values your magazine ascribes to the literary. This will form the background of our discussion on Thursday. Much information might be found in the MJP's introduction to the journal you're studying, in the Essays section, and in the Biographies area. Those interested in further research can check out the Books and Periodicals Database. I've added more practical information to the assignment page, so please do read it over again.
Also, since some of you expressed interest in technology workshops, use the comments here to (1) make requests, (2) indicate your availability, and (3) say whether you primarily use a Mac or a PC. I'll find out what facilities we can use at Brooklyn and will set something up.


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How These Car Parts Got Their Weird Names (Spoiler Alert: Horses Are Involved)
By Jennifer Gunner, M.Ed. Education , Staff Writer
Mother and daughter riding in vintage car
Siri Stafford / The Image Bank / Getty Images
You already know that brakes make a car stop and a steering wheel directs it where to go. You could probably even decipher that a muffler muffles the loud sounds emanating from a car engine. But do you know why your instrument panel is called a dashboard, or why a tire is a tire? It may seem like the names of car parts are random, but they all have an origin story — and it starts with a horse and a carriage.
The dashboard on your Tesla can do lots of things, but can it protect you from mud? Its 19th-century forefather certainly could. Back then, as a horse-driven carriage traveled along a muddy road, horses would kick up rocks and splash (or "dash") mud onto the unprotected carriage passengers. It didn't take long for drivers to install a board between the horses and the humans, known as a "dash-board," to serve the same purpose as a modern-day windshield or mud flap.
Dead Cat Hole
This one is just one of those morbid idioms, right? Sadly, no. There's a reason why the space between the tire and wheel well of a car is called the dead cat hole: Stray cats often sleep in this little space that is still radiating heat from the car's engine. However, if the cat's not too quick to awaken at the sound of the ignition … well, you get the picture.
Glove Compartment
Car registration, extra sunglasses, tissues, maybe a snack or two — you probably keep everything in your glove compartment except gloves. But the original glove compartment, which was a box stored on the floorboard of early automobiles, was designed to store driving gloves, because what uncultured monster would drive a car with their bare hands? The glove compartment moved from the floorboards to just below the dashboard, and the rest is (cluttered) history.
Close up grille of vintage car
Hans Neleman / Stone / Getty Images
Don't mix up a grill and a grille. One is for making delicious burgers and steaks, and the other keeps your engine cool by ventilating cool air through it. They both come from the Latin craticula ("gridiron"), but the meaning of grille has narrowed to only mean "an ornamental grating at the front of a car." Alas, until the automobile industry figures out how to safely install a barbeque grill in your car, the grille in the front is the only one you'll get.
"Pop the hood" is such a common automotive saying that we don't even think about how weird it sounds. It sounds even weirder in the U.K., where the covering over a car engine is called a bonnet, not a hood. But no matter what you call that big slab of metal, it's derived from older cars and their curved hoods' resemblance to a head covering. Modern car hoods are flatter, making the resemblance harder to see (unless your sweatshirt also has a wide, flat hood on it).
Hubcaps are those fancy-looking disks that keep your wheels from looking like they're about to fall off. While they're mostly decorative today, they used to serve an integral purpose on carriage wheels. Hubcaps (also called dust covers) covered the center hub of these wooden wheels, keeping them on their axles. Back then, a missing hubcap meant disaster; today, it's mainly a traffic faux pas.
Car aficionados know this one, but for everyone else, the rocker panel is not an intuitive part of the car. Which part rocks? Doesn't all of it rock? Like many other parts of a car, this one comes from old-timey carriages, specifically that part below the door and between the wheel wells that looked kind of empty behind a horse. Carriage designers added a rocker panel (think of that curved wooden plank that makes a rocking chair or rocking horse rock) to provide structural reinforcement and deflect rocks. And, of course, to look cute.
Old fashioned orange car with rear wind spoiler
Jean-Philippe Tournut / Moment / Getty Images
Spoiler alert! (Say that the next time you see a car with a big rear spoiler; ignore the pun-haters in the car.) The metal contraptions in the back of a car aren't just for show, and they aren't for ruining the plot of your favorite show, either — they're for reducing wind resistance around the car, also known as "spoiling" the airflow.
Have you ever taken a moment to wonder why those big rubber things attached to your car wheels are called tires? Is it because they're constantly moving and always get tired? Nope — tire is short for attire, meaning "a dressed wheel." Original tires used to be iron plates that covered a carriage wheel. In fact, that's where the term "tire iron" comes from. In this usage, they were known as tyres (and still are in England) until rubber tires were invented for bicycles in the late 19th century.
Last but not least is the most underappreciated part of your car: the trunk. So named because it used to be a literal traveling trunk strapped to the back of an early automobile, the trunk became an installed part of the car in the 1930s. But perhaps even more interesting is the origin of the British term for trunk, which is boot. In horse-drawn carriages, the coachman's seat (known as the "boot box," as it often stored boots) was in the back. "Boot box" became "boot," and thus, two very different words for the exact same thing were born.
More Mysteriously Named Items You Use Every Day
If you're ready to get out of the car, check out these explanations for the everyday things in your life you've never given a second thought about (but will now):
Snacks By Any Other Name: Brand Names and Their Origins
The Shoe-Stopping Origins Behind Your Favorite Shoe Brand Names
Your Shoe Has a What?! 'Aglet' & Other Words for Things You Didn't Know Had Names

redpajama_set_name: RedPajamaCommonCrawl


Cream Cheese Fruit Dip – Delicious, lightened-up creamy fruit dip made with cream cheese and plain yogurt. Simple, yet SO GOOD!
Light and creamy DIP that pairs perfectly with any fruit! This is possibly the best Fruit Dip I've ever made, and it's made with only 4 ingredients. The results are a super creamy and perfectly sweet Cream Cheese Fruit Dip.
Hi Hi!! It's MON-daaaaay! How in the world did it get here so fast?!? There I was dancing the night away on Saturday, and then the next thing I know it's Monday and my hangover is still here. Grrrr!
3 drinks you guys…. 3 MIXED drinks. Again, MIXED! That means, diluted alcohol… that means, I can't hang.
SO! HEY! How about them fruit dips!
Truth: I eat around 6 to 10 servings of fruit each day, and I do it without a Dip. Buuuuut… money says that if I had this dip every day, I'd eat 50 servings of fruit per day. IN fact, I could eat ONLY fruit and this Cream Cheese Fruit Dip for the rest of forever!
Okay, wait. That's pushing it. I also want tacos. AND Taratur. Bacon, too.
Strawberries are the perfect dipping fruit, right? Look at that! MMM!
I had the most amazing strawberries couple of weeks back. Juicy and super, super sweet. They didn't need a dip, but was I happy when I did pair them up with it. The strawberries were a 10 before that, yes, but slightly better with all that creaminess around them.
This sweet Dip exists somewhere in the world between a spread and a dip. Milk will help reach that desired consistency. It's definitely light, but rich, and a spoonful of sugar just makes the whole dang thing totally over the top.
You might consider sharing this with friends; it will make you even more popular! Take it from someone that knows!
If you love this recipe, you should also try my Frozen Yogurt Bark with Berries and/or my Cheesecake Bark with Chocolate Peanut Butter Swirl.
Delicious, lightened-up creamy fruit dip made with cream cheese and plain yogurt.
Place cream cheese in your mixer's bowl and beat on low speed until creamy and smooth.
Slowly add the yogurt and continue to beat until well combined.
Add brown sugar and vanilla; beat until combined and smooth.
Cover the dip and place in the refrigerator for 1 to 2 hours.
Remove from fridge and serve with fruit for dipping.
If you need to thin it out a bit, add a tablespoon of milk and stir until combined.
Awesome dip! I am I made this today, and I am planning to make it for a 4th of July party. I am making a platter of 4th of July- colored fruits, like apples, strawberries, and blueberries, and this dip is going to be a great addition in a cute 4th of July bowl! I love how light this dip is, I've tried to make other fruit dips in preparation for my party, but most other fruit dips are too dense and unpleasant to eat. Do you know how long this dip can sit in the refrigerator? For instance, could I make the dip at around 9:00 a.m, leave it to sit in the fridge, and serve it at about 5:00-6:00 p.m?
You can definitely leave it in the fridge for that long, even over night, but just mix it up when you take it out.
This Cream Cheese Fruit Dip looks and sounds incredible! Thanks for sharing I ran across this, plus many many more amazing recipes that you have on your Blog.
What a shame so many people still fall for the low-fat nonsense. Sugar and carbs are WAY worse for your waistline. I will make this with full fat ingredients and probably a low cal sweetener, stevia or monkfruit so all the artificial sweetener nazis don't get in a twist.
I can't seem to get enough of fruit dips when I make them! Theyre perfect for weekend guests and for snacking.
Ive actually never made a sweet dip before for some reason – so thanks for this idea! I definitely have to make the recipe.
oh wow that dip looks amazing I think I will need extra strawberries!
I'm loving this lightened up version!
I thought I was the only one that devoured fruit and if I had this dip, I would eat a million more too! Is by the spoonful okay?!
This sounds amazing! Instead of the strawberries, can I just dip my face in it?
Mmm..Now I want to dip all the things in this fruit dip!
Wow! Beautiful photos! I am working with a specific maple syrup brand right now, and I want to try mixing one of their flavours into your recipe! Looks so good!
Omg, this cream cheese fruit dip sounds so delicious. I think we're definitely going to have to try this. Thank you for posting this recipe.
Hahaha I hear ya!! I've made a rule with myself the older I get, three drinks max! Anything after that leaves me in bed for the better part of the next day….
I'm not alone!! LOL!!! This is insane…all I want to do is sleep! haha 😀 Thank you, Nicole!


During a free day you might choose to explore your lovely base, Minori, or simply soak up the sun by your hotel's swimming pool. Alternatively you can join an optional excursion to discover the exceptional archaeological site of Pompeii, the Roman town frozen in time by the eruption of Mount Vesuvius in 79 AD. You're going to explore in fantastic company, as a Local Guide leads you through its maze of streets. As you stroll you'll get a fascinating insight into the last days of the people who lived here. You'll see villas still decorated with brightly painted mosaics, Roman baths and an impressive amphitheatre. There are even bakeries here that still have their bread ovens and flour grinders intact.
Naples- 56.5 km – 1 hour 30 minute drive approx.
Sorrento – 35.7 km- 1 hour 28 minute drive approx.
Amalfi- 3.9 km- 12 minute drive approx.
Pre-bookable excursions: The above optional excursions can be pre-booked as a package from just £189 per person.


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Wimbledon 2018 | Djokovic ousts Edmund in controversial third round clash
By Ros Satar, at Wimbledon
Novak Djokovic [12] def. Kyle Edmund [21] 4-6 6-3 6-2 6-4
WIMBLEDON, UK – Novak Djokovic continues to look like a strong contender as he beats British No. 1 Kyle Edmund to reach the second week.
CLICK TO BUY FROM THE WIMBLEDON SHOP
British No. 1 Kyle Edmund's campaign at Wimbledon came to an end at the hands of three-time Wimbledon champion Novak Djokovic.
The start of the match, straight after England's World Cup triumph to reach the semi-finals, saw a buoyed-up Edmund impress the crowd with improved movement and a stronger backhand this season, first fending off break points and then finally converting on a fourth chance of his own to take a 4-3 lead, hanging on to that advantage to the end of the set.
Edmund stayed firm against Djokovic's early attempts to break him but could not quite hold on as the Serbian broke towards the end of the set, serving out to level the match.
The Brit was broken early at the start of the third set, as the crowd started to get to Djokovic, laughing at faults, booing him as he started his ball-bouncing pre-serve routine, which served to fire him up all the more, indicating to the crowd that he couldn't hear them, after he broke Edmund once more and served to love for a 2-1 lead.
There was more drama to come as Edmund fended off break point chances including a controversial call where a double-bounce which eventually was actually out, but the point was awarded to Edmund, much to Djokovic's frustration.
In fact if anything, fans on twitter were more annoyed with Edmund for not owning up to the double-bounce. In the end though, Djokovic was rewarded with the break before serving out to love to book his place in the Round of 16.
From Djokovic's perspective, he likened it to a Davis Cup envionrment but did point out that certain members of the crowd were deliberately trying to goad him.
He said: "I played Andy couple times. I played him Olympic Games. I played him Wimbledon. It was not like this, definitely. The crowd was very fair when I played against Andy. Obviously they support their player. There's nothing you can say about that. Of course, I mean, it's expected.
"But today there was just some people, especially behind that end where I got the time violation, they kept on going, they kept on going, provoking. That's something that I can tolerate for a little bit, but I'm going to show that I'm present, as well, that they can't do whatever they feel like doing.
"I didn't deserve to be treated as I was treated by certain individuals. That's one thing I didn't like."
As if that had not been bad enough, his frustration had grown with the situation surrounding the double-bounce.
He explained: "It was quite a strange situation. First of all, I mean, the only thing I wanted to know from him is, how does he think it's possible that Kyle hits the shot that he hit so clean and so flat and fast if he hit it with the frame. If you hit it with the frame, it's supposed to kind of slow down the trajectory of the ball. I was 100% convinced it was twice. I heard from people that it was.
"Anybody can make a mistake. That's okay. But I don't understand why he didn't allow me to challenge the ball. I asked him.
"At first, obviously I didn't like his call. I had a conversation with him. I understand it took some time. But I wanted to challenge the call. If I couldn't change the decision, I just wanted an explanation. Then I said, Okay, can I challenge the call? He said, It's too late. So yes, it was quite a strange decision from chair umpire, but it happens."
Edmund came in for quite a lot of criticism on Twitter during the match after that incident, but in the heat of the moment, Djokovic believed that he had not known about the ball hitting the ground twice.
"I don't think he deserves that. Kyle is a very nice guy. I know him and have tons of respect for him, his team. We get along very well. Nothing against Kyle there. You couldn't know. I mean, he was running towards the ball and he just hit it and he dropped his racquet. He couldn't know. Doesn't deserve that."
Edmund admitted he had been scrambling for the ball at the time so asserted that it was hard to say if it had double-bounced or not, despite it having been proved so via a television replay.
Edmund said: "I was scrambling. I mean, it sounds like you're still unsure if it bounced twice.It's hard to say, isn't it? That's the thing. You need television to see it. If in real life it's hard to tell, then it's hard to tell for me when I'm scrambling.
"Generally, if you need television to look at stuff, when you're in the moment trying to make that split decision… I don't really know what to say. I try my best to get there. We need the umpire to get off his chair and go to the TV monitor on the side."
Wimbledon continued with all the fourth round matches scheduled on Monday.
CLICK TO BUY PLAYER GEAR FROM PRO-DIRECT TENNIS via Britwatch Sports
kyle edmundNovak DjokovicWimbledon
Wimbledon 2018 | 'Tired' Halep exits in first week, as nine of Top 10 seeds fail to make fourth round
Wimbledon 2018 | Three to See on Day 7


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Hawk Central
All Iowa Sports Awards
Iowa State women's basketball's Stephanie Soares getting strong support during time of uncertainty
Tommy Birch Des Moines Register
AMES – Iowa State coach Bill Fennelly and some members of the Cyclones women's basketball team have just finished interviews with local media when post player Stephanie Soares emerges from the locker room.
Soares, who was usually front and center for these gatherings, walks out as a school official puts away an Iowa State backdrop that's set up for the press conferences.
"It's kind of been challenging," Soares says of how things have changed.
A lot has happened over the last month for the graduate transfer senior. Soares was having huge success in her first season in Ames before she sustained a season-ending knee injury Jan. 8 vs. Oklahoma.
"It's funny how you miss something more after you lose it," Soares said.
While Iowa State moves forward with it season, all Soares can do is watch and cheer on her teammates. Soares will undergo surgery for her torn ACL on Thursday, and she hopes to get back on the court again and be the player she was before she got hurt.
"We can't really say for sure what's going to happen in the future," said her father, Rogerio Soares. "But we know for sure that's she's working to continue playing basketball at another level."
Soares' stock was soaring and the Cyclones were rolling. Then she got hurt
Soares made an instant impact at Iowa State as s 6-foot-6 forward/center. The Cyclones, who had been to the Sweet 16 the season before, needed some size and strength in the post to take them to the next level. Soares was the perfect fit. She was a two-time NAIA Player of the Year and a star at The Master's.
Soares successfully made the jump from NAIA to the Big 12 Conference. She earned a starting spot right away and became a star, averaging 15.4 points, 10.8 rebounds and 3.17 blocks per game. Fennelly said pro teams had her on their radar as she helped Iowa State to a 10-2 start.
"I was just focusing on getting better every single game and working on different things I needed to work on," Soares said.
But everything changed in the Oklahoma game. Carolyn Peck, a former college and WNBA coach who was calling the game for ESPN2, was gushing about Soares' season when the Cyclones star took a shot and landed awkwardly. She grabbed her left knee.
"I knew right away," Soares said.
Soares suffered the same injury to the same knee while playing at The Master's. But this time there was more at stake. The Cyclones lost a rare player with the skillset to dominate in the paint and knock down the 3. Then there was Soares' pro future to think about. Several teams attended the game at Oklahoma to watch Soares. Now, everything was in doubt.
"You kind of plan one way but now you kind of have to think differently," her mother, Susan Soares, said.
What's next for Soares? WNBA teams are keeping close tabs on her
Fennelly said he's heard from every WNBA team. They all wanted to check in to see how Soares is doing. Some wanted updates about when she'll have surgery and what the road to recovery looks like.
Fennelly said he's told WNBA teams that Iowa State is putting in a waiver to try to gain Soares another season of eligibility because of the injury. Soares is unsure if she would return to college if the waiver is approved. Fennelly said a WNBA team could draft her in 2023 and secure her rights while she rehabs. He said a typical road to recovery takes nine to 12 months.
"If she wants to be a pro, that's going to be right in the middle of her rehab," Fennelly said. "So, we need to make sure that we have everything ready for whatever she decides because our No. 1 responsibility is to fix her Thursday and get her rehabbed so the next time she steps onto the basketball court, wherever it is, she's ready."
Soares is doing some biking exercises and pool workouts. Thursday's operation will help doctors discover just how bad the damage is and how much time she'll need before resuming basketball activities.
Soares misses being on the court. But she's still with her teammates at practice to cheer them on and to help her replacements, Morgan Kane, Nyamer Diew and Izzi Zingaro. Soares said Iowa State fans have dropped off notes of encouragement for her at Hilton Coliseum. Kansas State coach Jeff Mittie brought her a hand-written note when his team came to Ames. Texas coach Vic Schaefer did the same. Soares also received flowers from an opposing team. Her parents have sent her Bible verses. Everything helps.
"It's great to have that support," Soares said.
Soares wants to play at the next level and will do whatever it takes to get back.
"That's the plan," she said. "So, we'll see."
Tommy Birch, the Register's sports enterprise and features reporter, has been working at the newspaper since 2008. He's the 2018 and 2020 Iowa Sportswriter of the Year. Reach him at tbirch@dmreg.com or 515-284-8468. Follow him on Twitter @TommyBirch.