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Джон О'Мэлли (; ) — американский католический , священник-иезуит; специалист по религиозной культуре Европы раннего нового времени, особенно Италии. Доктор философии, Университетский профессор Джорджтаунского университета, где преподавал с 2006 года, член Американского философского общества (1997). Труды удостаивались отличий. Вероятно, самая известная работа — The First Jesuits (Cambridge, MA: Harvard University Press, 1993) — была переведена на 12 языков.

Был единственным ребенком в семье; по отцовской линии, несмотря на ирландскую фамилию, их семья была преимущественно немецкой. В школьные годы определился с тем, чтобы стать священником.
В 18-летнем возрасте присоединился к иезуитам, стал новициатом в 1946 году и был рукоположен в 1959 году. Вспоминал, что во время своего пребывания в Австрии «понял, насколько важно интегрировать церковную историю со светской и культурной историей».
Степень доктора философии по истории получил в Гарвардском университете, учился там в частности у . 14 лет преподавал в Детройтском университете.

В 2020 году ушел в отставку из Джорджтаунского университета. Член Американской академии искусств и наук (1995).
Являлся президентом  (1998). C 2010 по 2016 год вице-президент Американского философского общества. Умер от рака. Как исследователь он отмечал: «Стиль — это не просто украшение мысли, а выражение смысла». О'Мэлли также любил говорить: «Традиция не инертна, а динамична»; а еще высказывался: «Историки всегда должны смотреть на непрерывности и трещины: на мой взгляд, непрерывность всегда глубже, чем любые разрывы». Называл своим хорошим другом .

Автор 14 книг и редактор восьми. Из своих трудов своим «любимым дитем» называл Praise and Blame in Renaissance Rome.

Примечания

члены Американского философского общества
доктора философии по истории


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\section{Introduction}
Violations~\cite{Haugan1979,Damour1996,Will2014,Hees2018} of the Einstein equivalence principle (EEP)~\cite{Einstein1905,Einstein1907,DiCasola2015} and the existence~\cite{Damour1990,Boehm2004} of dark matter could be explained by scalar, light dilaton fields~\cite{Alves2000,Damour2010,Damour2012}.
They can be motivated by String Theory~\cite{Damour1994} and influence the propagation of light and matter, leading to deviations from established laws of physics.
While effects on matter have been thoroughly discussed~\cite{Damour1999,Arvanitaki2015,Geraci2016,Arvanitaki2018,Hees2018,ElNeaj2020,Roura2020,Roura2020b,Ufrecht2020,Badurina2021,DiPumpo2021,Zhao2021}, we focus on the electromagnetic field interacting with the dilaton and study the detection of dilaton fields by light-pulse atom interferometers~\cite{Kasevich1991,Cronin2009}.

While more advanced models are possible~\cite{Will2014}, the dilaton field already captures EEP violations and dark-matter effects, i.e., signatures of physics beyond the Standard Model and general relativity.
The dilaton field can be influenced by the presence of large masses like Earth, and thus induce violations of the universality of the gravitational redshift (UGR) and of free fall (UFF), as detected by EEP tests~\cite{Pound1960,Hafele1972a,Hafele1972b,Vessot1980,Godone1995,Fray2004,Chou2010,Bonnin2013,Schlippert2014,Ashby2018,Zhang2018,Delva2019,Touboul2019,Savalle2019,Asenbam2020,Takamoto2020,Bothwell2021}.
Additionally, an oscillating background field of cosmic origin can serve as a simple model for dark matter and gives rise to oscillating fundamental constants~\cite{Damour1999,Arvanitaki2015,Arvanitaki2018}, like the fine-structure constant.
Since the internal atomic structure depends on the value of these constants, atomic clocks~\cite{Moller1956,Katori2003,Nicholson2015,Brewer2019,Madjarov2019,Oelker2019} can be used to search for EPP violations~\cite{Damour1999,Hees2018} and dark matter~\cite{Arvanitaki2015,Derevianko2018,Wcislo2018}.
Similarly, in light-pulse atom interferometers~\cite{Kasevich1991,Cronin2009,Kleinert2015} matter propagates within dilaton fields and consequently such devices are susceptible~\cite{Tino2021} to both EPP violations~\cite{Giulini2012,Roura2020,Roura2020b,Ufrecht2020,DiPumpo2021} and dark matter~\cite{Geraci2016,Arvanitaki2018,ElNeaj2020,Badurina2021}.
However, with light pulses being an essential tool to manipulate the atoms, their modified behavior in gravity~\cite{Einstein1911,Tsagas2004,Bruschi2014,Cabral2017,Exirifard2021,Exirifard2021b,Mavrogiannis2021} and dilaton fields has to be taken into account for a consistent description of such experiments.

In this article we show that the propagation of light in dilaton fields has to lowest order no influence on the signal of an atom interferometer, while gravity leads to a modified momentum transfer.
Indeed, the dominant dilaton contribution to the interference pattern originates from the propagation of matter in the dilaton field.
To showcase the combined influence of light propagation and dilaton on atom interferometers, we study different schemes including gradiometers, EEP tests, and dark-matter detectors.
For the latter, we consider the spatial dependence of the dilaton field and discuss its consequences, which was not taken into account in previous treatments~\cite{Geraci2016,Arvanitaki2018,ElNeaj2020,Badurina2021}.

\section{Modified Maxwell equations}
We consider a classical dilaton field coupling linearly to all particles and forces in the Standard Model~\cite{Damour1994,Alves2000,Damour2010,Damour2012}.
The modified Lagrangian density for the electromagnetic sector is
\begin{align}
	\begin{split}
		\label{eq:DilIntLagFree}
		\mathcal{L}_\text{EM}=-\frac{\sqrt{-\mathfrak{g}}}{4\mu_0}(1-\varrho d_e)F_{\mu\nu}F^{\mu\nu},
	\end{split}
\end{align}
which includes a linear coupling between the dilaton field $\varrho$ and the electromagnetic field strength tensor $F_{\mu\nu}=\nabla_{\mu}A_\nu-\nabla_{\nu}A_\mu=\partial_{\mu}A_\nu-\partial_{\nu}A_\mu$ with coupling constant $d_e$ and vacuum permeability $\mu_0$.
Here, we introduced the determinant $\mathfrak{g}$ of the metric tensor, the covariant derivative $\nabla_\mu$, the partial derivative $\partial_\mu$, as well as the four-vector potential $A_\mu$.
The variation of this Lagrangian density with respect to $A_{\nu}$ leads to the Euler-Lagrange equation
\begin{align}
	\begin{split}
		\frac{\partial\mathcal{L}_\text{EM}}{\partial A_{\nu}}=\nabla_{\mu}\left(\frac{\partial\mathcal{L}_\text{EM}}{\partial(\nabla_{\mu}A_{\nu})}\right),
	\end{split}
\end{align}
which gives rise to modified Maxwell equations.
Making use of the identity $\nabla_{\mu}\sqrt{-\mathfrak{g}}=0$, we find
\begin{align}
	\begin{split}
		\nabla_{\mu}(1-\varrho d_e) F^{\mu\nu}=0
	\end{split}
\end{align}
valid in the absence of four-currents, i.e., $\partial\mathcal{L}_\text{EM}/\partial A_{\nu}=0$~\footnote{The same result can be obtained from a similar variation with respect to $\partial_\mu A_\nu$ instead of $\nabla_{\mu}A_\nu$}.
Since the dilaton does not alter the metric tensor to lowest order (see Appendix~\ref{sec:App}), it can still be used to transform co- into contravariant quantities and vice versa.
Furthermore, adding a gauge field to the vector potential leaves the field strength tensor invariant and gauge freedom allows choosing the modified Lorenz gauge $\nabla_{\mu}(1-\varrho d_e)A^{\mu}=0$.
Together with the identity $\nabla_{\mu}\varrho=\partial_{\mu}\varrho$ and the Ricci tensor $R^\nu_\sigma$, we find the Maxwell equations
\begin{align}
	\begin{split}
		\nabla_{\mu}\nabla^{\mu}A^\nu=R^\nu_\sigma A^\sigma+(\partial_{\mu}\varrho)d_e\nabla^{\mu}A^\nu+	\nabla_\mu(\partial^\nu\varrho)d_e A^\mu,
	\end{split}
\end{align}
neglecting orders of $d^2_e$.
In the following, we consider a metric $\mathfrak{g}_{\mu\nu}=\eta_{\mu\nu}+\delta^0_\mu\delta^0_\nu 2 g z /c^2$ with gravitational acceleration $g$ pointing in $z$ direction and with  $R^\nu_\sigma=0$.
Here, $\delta_\mu^{\nu}$ is the Kronecker delta and $\eta_{\mu\nu}$ the Minkowski metric.
We keep only terms of order $g z/c^2$ as well as $d_e$, omitting higher contributions in the slowly-varying and weak-field limit for the source mass-energy density.
In Appendix~\ref{sec:App}, the metric is derived together with the solution for the dilaton field under the assumption of a source mass-energy density homogeneously distributed over an infinite plane.

We rely on the geometrical-optics ansatz~\cite{Dolan2018,Bartelmann2019,Linnemann2021}
\begin{align}
	\begin{split}
	A^{\nu}=\left(a^\nu+\epsilon b^\nu\right)\text{e}^{-\text{i} \Phi/\epsilon}+\mathcal{O}\big(\epsilon^2\big)
	\end{split}
\end{align}
to obtain propagating-beam solutions to the Maxwell equations.
In this approximation we assume that $\Phi$ is of order unity so that the factor $\exp{(-\text{i}\Phi/\epsilon)}$ varies fast compared to the amplitude $a^\nu$ and is common for all four components of the vector potential.
By combining the radiation wavelength $\lambda$ and the typical length scale $L$ of light propagation, we form a small parameter $\epsilon=\lambda/L$ for the perturbative solution of the Maxwell equations~\footnote{For more general situations where also a curvature is included into the metric, we generalize the definition to $\epsilon=\lambda/\min{(L,\mathcal{C})}$. Here, $\mathcal{C}\sim 1/\sqrt{\max{\left|R_{\mu\nu\kappa\sigma}\right|}}$ is the curvature radius scale.}.
For red laser light around $\lambda \sim 700$\,nm and for distances of $L\sim 1$\,mm, both typical scales for atom interferometry, we find $\epsilon= 7\cdot 10^{-4}$.
In more ambitious atom-interferometric setups, larger distances or different wavelengths give rise to an even more suitable regime.
After applying the perturbative expansion the factor $\epsilon$ can be absorbed into a redefinition of the wave vector.

When we define the wave vector $K_\mu=\partial_\mu \Phi$ and insert the ansatz into the Maxwell equations we obtain to leading order in $\epsilon^{-2}$ the condition $K_\mu K^\mu=0$.
This expression directly implies the eikonal equation
\begin{align}
	\begin{split}
	\mathfrak{g}^{\mu \nu}\partial_\mu \Phi\partial_\nu\Phi=0.
	\end{split}
\end{align}
As a consequence, the phase is independent of the dilaton field $\varrho$.
Since the metric only depends on the $z$ direction, we make the ansatz $\Phi=ck_0t-k_x x-k_y y-\kappa(z)$ to separate variables with $\kappa(0)=0$ and constants $k_0$, $k_x$ and $k_y$.
In the following, we define $\boldsymbol{q}=(k_x,k_y)^{\text{T}}$ and $\boldsymbol{r}=\left(x,y\right)^{\text{T}}$.
Together with the eikonal equation, we find $\kappa(z)=k_z\big[1-gk_0^2z/(2c^2k^2_z)\big]z$ for real constants $k_z$ and $k_0^2=\boldsymbol{q}^2+k_z^2$.
We observe that the phase of the electromagnetic field in $z$ direction, and thus also the wave vector, are modified by gravity via the additional term $gk_0^2z^2/(2c^2k_z)$.
The phase $\Phi$ is shown in the spacetime diagram of Fig.~\ref{fig:PhaseAndAmplitude}\hyperref[fig:PhaseAndAmplitude]{(a)}, where we also plot the wave vector $K_\mu$ as a vector field along a light cone of constant phase.
The light cone is deflected by gravity compared to the flat-spacetime case, but experiences no effect caused by the dilaton.
The figure also shows the change of the $z$ component of the wave vector along the light cone.
\begin{center}
\begin{figure}[h]
	\includegraphics[width=1\columnwidth]{PhaseAmplitude.pdf}
	\caption{Effects of gravity and dilaton on the propagation of the electromagnetic field:
	The density plot (a) displays the scaled phase $\Phi/(k_z L)$ in a spacetime diagram, where $L$ is a typical length scale of the experiment.
	A light cone defined by a plane of constant phase (white curve) is deflected by gravity compared to the gravity-free case (dashed white line).
	The four-wave vector $K_\mu$ is the gradient of the phase and therefore orthogonal to the light cone.
	The two relevant components  $(K_0,K_z)$ are denoted by white arrows.
	As expected, the dilaton has no influence on the phase and the wave vector.
	A plot of the decreasing $z$ component $-K_z/k_z$ along the light cone is shown on the bottom.
	The amplitude $a/a_\text{in}-1$ is displayed by the density plot in panel (b) in a spacetime diagram.
	Again, we include the light cone (white curve) and the four-wave vector $K_\mu$ (white arrows) for reference.
	Although the phase and wave vector are not influenced by the dilaton, the underlying amplitude is modified by gravity and by the dilaton field with its oscillating background term.
	To highlight this effect, a cut of the oscillating amplitude along the light cone is shown on the bottom.
	For all plots, we use the exaggerated values $g L /(2c^2)= 0.2$, $d_e \bar{\beta}_\text{S}=0.3$, $d_e \bar{\varrho}_0= 0.02$, $k_\varrho L = 5$, $\omega_\varrho L /c = 40$, $\phi_\varrho = 0$, and $\boldsymbol{q}=0$ to enhance the visibility of the effect.}
\label{fig:PhaseAndAmplitude}
\end{figure}
\end{center}

Conventionally, one separates $a^\nu=a e^\nu$ into real amplitude $a=\sqrt{a^*_\nu a^{\nu}}$ and complex polarization $e^\nu$ with $e^*_\nu e^{\nu}=1$.
To order $\epsilon^{-1}$ we find from the gauge condition that $K_\mu e^\mu=0$, which implies an orthogonality between wave vector and polarization.
With this result, we find from the Maxwell equations to order $\epsilon^{-1}$ the equations of motion
\begin{align}
        \begin{split}
		&K^\mu\partial_\mu a+\frac{a}{2}\left[\nabla_\mu-\big(\partial_\mu\varrho\big)d_e\right]K^\mu=0,\\
		&K^\mu\nabla_\mu e^\nu=0
		\end{split}
\end{align}
for amplitude $a$ and polarization $e^\nu$, respectively.
Therefore, the dilaton modifies only the scalar amplitude but not the polarization.
To solve these equations, we use the explicit form of the Christoffel symbols included in the covariant derivative as well as the specific form of the dilaton field.
For the metric linear in $z$ we find $\Gamma^\nu_{0\lambda}=g(\delta^\nu_0 \delta^z_\lambda+\delta^\nu_z \delta^0_\lambda)/c^2$ and $\Gamma^\nu_{j\lambda}=\delta^\nu_0\delta^z_j \delta^0_\lambda g/c^2$.
Moreover, the dilaton field $\varrho=\bar\varrho_0\cos{\left(\omega_\varrho t-k_\varrho z+\phi_\varrho\right)}+\bar\beta_\text{S}g z/c^2$ arises for a homogeneously distributed mass-energy density, see Appendix~\ref{sec:App}.
Here, $\bar\beta_\text{S}$ corresponds to the linear expansion coefficient of the source mass $m_\text{S}$ of the gravitational field around its Standard-Model value, while $\bar\varrho_0$ is a perturbative amplitude.
The plane-wave part of the dilaton field has a frequency $\omega_\varrho$, an initial phase $\phi_\varrho$, and a wave number $k_\varrho$.
Thus, the dilaton field is a superposition of a contribution caused by the source mass and an oscillating background part.
As a consequence of these considerations, the components $e^x$ and $e^y$ of the polarization in $x$ and $y$ direction are constant and given by their initial values.
In contrast, for the other directions of the polarization we obtain
\begin{align}
	\begin{split}
		&e^0(z)=e^0_\text{in}\left[1-\frac{g z}{c^2}\right]-e^z_\text{in}\frac{g z}{c^2}\frac{k_0}{k_z}, \\
		&e^z(z)=e^z_\text{in}-e^0_\text{in}\frac{g z}{c^2}\frac{k_0}{k_z},
	\end{split}
\end{align}
where $e^\nu_\text{in}$ denotes the initial value of each component.
Moreover, to lowest order in all perturbative parameters, neglecting cross terms, the amplitude
\begin{align}
\begin{split}
    a(z,t)=a_\text{in}&\left[1+\frac{g z}{2 c^2}\left(\frac{\boldsymbol{q}^2}{k^2_z}+d_e\bar\beta_\text{S}\right) +\left(1-\frac{\omega_\varrho}{ck_\varrho}\frac{k_0}{k_z}\right)\right.\\
    &\left.\times d_e\bar\varrho_0\sin{\left(\frac{k_\varrho z}{2}\right)}\sin{\left(\omega_\varrho t-\frac{k_\varrho z}{2}+\phi_\varrho\right)}\right]
\end{split}
\end{align}
with real initial value $a_\text{in}$ depends on time and position.
Since the square of the amplitude $a(z,t)$ is proportional to the energy density, we observe that it also depends on the dilaton and by that on time.
This effect can be directly seen in Eq.~\eqref{eq:DilIntLagFree} from the modification of the Lagrangian density $\mathcal{L}_\text{EM}$ by the dilaton field.
For $k_0=k_z$ and vanishing dilaton mass $m_\varrho$, the time-dependent dilaton modification to the amplitude ceases to exist.
As expected from the $z$ dependence of the metric, the polarization only changes in vertical direction (and only via the metric tensor, not influenced by the dilaton).
In Fig.~\ref{fig:PhaseAndAmplitude}\hyperref[fig:PhaseAndAmplitude]{(b)} we plot the amplitude of the electric field in a spacetime diagram.
The light cone and wave vector $K_\mu$ from Fig.~\ref{fig:PhaseAndAmplitude}\hyperref[fig:PhaseAndAmplitude]{(a)} are included for reference.
We observe that the field experiences different amplitudes for different points in spacetime, depending on gravity and the underlying dilaton field.
Moreover, we illustrate this effect with the cut of the amplitude along the light cone shown on the bottom.

Since the electric field is obtained by taking the derivative of the vector potential, its phase corresponds to the same one as of $A^\nu$.
This fact implies that the frequency of the electric field $c k_0$ is independent of the position within the chosen frame of reference, and displays no gravitational modification.
In particular, this frequency experiences to leading order no modifications from the dilaton, which are only included in the amplitude of the electric field.
For illustration, we imagine two fixed atomic clocks at different heights that probe for violations of the gravitational redshift~\cite{Pound1960,Chou2010,Takamoto2020,Bothwell2021}.
The initialization and readout of these clocks is performed with light pulses.
During the interaction, the phase of the electric field is imprinted onto the atoms.
As a central result we find that this phase is independent of the dilaton field, and possible violations of the gravitational redshift measured by these clocks arise due to the coupling of matter to gravity and the dilaton field, and not from the modified phase of the electric field itself.

Conventionally, clocks are based on recoilless internal transitions~\cite{Alden2014,Bothwell2021} during the initialization and readout process.
However, for general pulses, the momentum of light carried by the wave vector cannot be neglected, and experiences a gravitational modification.
The absorption and emission process causes a recoil of the first-quantized atom with center-of-mass position operator $(\hat{\boldsymbol{r}},\hat{z})^{\text{T}}$.
It is usually encoded~\cite{Kleinert2015} in the mode function $\exp{\big(\pm \text{i}\left[\boldsymbol{q}\hat{\boldsymbol{r}}+k_z\hat{z}\right]\big)}$ that gives rise to the momentum displacement $\pm (\hbar\boldsymbol{q},\hbar k_z )^\text{T}$.
However, this displacement operator is modified to $\exp{\big(\pm \text{i} [\boldsymbol{q}\hat{\boldsymbol{r}}+k_z  \hat{z}-gk_0^2\hat{z}^2/(2c^2k_z) ]\big)}$ in the presence of gravity.
Since setups like atom interferometers are built on this momentum transfer, there is an effect due to the altered wave vector.

\section{Atom-interferometric experiments}
For the following calculations, we restrict ourselves to unidimensional interferometer setups in $z$ direction and thus choose $\boldsymbol{q}=0$ and $k_0=k_z$.
Conventionally, atom interferometers are operated via two-photon processes like Raman~\cite{Kasevich1991,Hartmann2020} or Bragg~\cite{Torii2000,Giese2015} diffraction, but recently single-photon diffraction has also gained some attention~\cite{Hu2017,Rudolph2020}.
Two-photon transitions usually involve a red-detuned laser with $k_z^\text{R}$ and a counterpropagating blue-detuned laser with $k_z^\text{B}$.
Both wave vectors are defined by their respective value at the surface of the source mass, i.e., $z=0$.
They give rise to the differential phase of both light fields $\Phi_B-\Phi_R=\Delta \omega t-kz\big[1-gz/(2c^2)\big]$.
Here, $\Delta\omega=c(k_z^\text{B}-k_z^\text{R})$ is the frequency difference and is proportional to the transferred energy during resonant diffraction, whereas $k=k_z^\text{B}+k_z^\text{R}$ is the effective wave vector transferring momentum, which experiences a modification by the factor $1-gz/(2c^2)$.
Thus, the gravitationally modified wave vector for a two-photon process has the same form as the one from a single-photon process, even though $\Delta\omega$ and $k$ can be tuned independently.
Figure~\ref{fig:MZI}\hyperref[fig:MZI]{(a)} illustrates the impact of the modified wave vector on the red and blue lasers involved in a two-photon process via arrows with different lengths.
\begin{figure}
	\centering
	\includegraphics{mzi.pdf}
	\caption{Effects of perturbations on atom interferometers:
	In (a) we depict diffraction from two counterpropagating light fields with different colors.
	We illustrate the opposite contractions of the blue and red wave vectors $K^\text{B}_z$ and $K^\text{R}_z$, originating from the propagation in different directions.
	As a consequence, they lead to a modified effective wave vector $k\big[1-gz/(2c^2)\big]$.
	A complete Mach-Zehnder sequence is shown in (b), where an initial $\pi/2$ pulse creates a spatial superposition, redirected by a $\pi$ pulse after time $T$, and brought to interference by a final $\pi/2$ pulse after another time interval $T$.
	Here, we draw the unperturbed atomic trajectories but highlight the effects due to perturbations.
	These perturbations include the modified wave vector of the effective pulse represented by the curved red light cones due to $k\big[1-gz/(2c^2)\big]$.
	The inset lenses illustrate that the diffracting wave vectors change for different pulses.
	Moreover, the finite speed of light leads to a delay of order $\delta z/c$ between the diffraction of the lower and the upper branch for the $\pi$ pulse.
	Finally, we also include the coupling of the atom's mass $m$ to the dilaton field by two aspects: the mass-dependent gravitational acceleration $\beta g$ and the oscillating background represented by the shading between white and yellow.}
\label{fig:MZI}
\end{figure}
We neglect the motion of the atom during the pulse, which corresponds to a vanishingly small pulse duration compared to the duration of the interferometer.
In this case, the interferometer can be described by a series of instantaneous momentum transfers with the effective potential
\begin{align}
\label{eq:kick-potential}
    \hat{V}=-\hbar\sum_n{k_n\hat{z}\left[1-\frac{g\hat{z}}{2c^2}\right]\delta(t-t_n)}= \hat{V}_0+\hat{\mathcal{V}},
\end{align}
where the momentum transfer $\hbar k_n$ of the $n$th light pulse at time $t_n$ is modified by gravity.
The time evolution with this potential directly modifies the displacement operator to the operator introduced in the preceding section.
Moreover, the second term in the brackets, defined as $\hat{\mathcal{V}}$, can be interpreted as a small perturbation to the momentum transfer without gravity included in $\hat{V}_0$.
The dilaton-dependent amplitude of the vector potential only leads to a modified Rabi frequency and, therefore, does not contribute to the momentum transfer to first-order perturbation theory.

However, the dilaton indeed contributes to the phase of an atom interferometer~\cite{Geraci2016,Arvanitaki2018,ElNeaj2020,Roura2020,Roura2020b,Ufrecht2020,Badurina2021,DiPumpo2021,Zhao2021} because the complete Hamiltonian for a particle of mass $m$ and momentum $\hat{p}$ is
\begin{align}
\label{eq:Hamiltonian}
\begin{split}
    \hat{H}^{(\sigma)}=&m c^2 +\frac{\hat{p}^2}{2m}+m g\hat z +\hat{V}^{(\sigma)}_0\\
    &+\hat{\mathcal{V}}^{(\sigma)}+m g\beta\hat z+ m c^2\varrho_0\cos{\left(\omega_\varrho t-k_\varrho\hat{z}+\phi_\varrho\right)}
\end{split}
\end{align}
and depends on the dilaton parameters $\beta=\bar\beta\bar\beta_\text{S}$ and $\varrho_0=\bar\beta\bar\varrho_0$.
It leads to a particle-dependent gravitational acceleration $g(1+\beta)$ for the center-of-mass motion between the pulses, introducing EPP violations~\cite{Damour1999,Giulini2012,Hees2018,Roura2020,Roura2020b,Ufrecht2020,DiPumpo2021,Fray2004,Zhang2018}.
The Hamiltonian also includes time-dependent modifications caused by the dilaton field that are independent of gravity, which can be connected to dark matter~\cite{Arvanitaki2015,Geraci2016,Arvanitaki2018,ElNeaj2020,Badurina2021}.
Here, we anticipated that an atom interferometer consists of at least two branches by introducing the superscript $\sigma = u, l$ for the upper and lower branch.
They are generated by branch-dependent momentum kicks $\hbar k^{(\sigma)}_n$ encoded in $\hat{V}^{(\sigma)}$ as a generalization of Eq.~\eqref{eq:kick-potential}.
The dilaton parameter $\bar\beta$ effectively corresponds to the linear expansion coefficient of the mass $m$ around its Standard-Model value.

Our goal is to identify the leading-order contributions of the dilaton field and the propagation of light, including its finite speed, to the signal of atom interferometers.
To keep focus, we neglect other effects in our description, such as relativistic kinetic corrections, possibly in the same order of magnitude.

To compute phases in dilaton gravity, we consider the Bragg-Mach-Zehnder~\cite{Torii2000} geometry shown in Fig.~\ref{fig:MZI}\hyperref[fig:MZI]{(b)}, where in contrast to Raman-based schemes the pulses induce no internal transitions.
The figure highlights the impact of the modified potential by curved light cones representing effective Bragg pulses, and arrows with different lengths at two interaction points transferring position-dependent momentum.
Moreover, we also indicated the perturbations from finite speed of light, modified wave vectors, and dilaton fields described in more detail below.
The scheme consists of an initial $\pi/2$ light pulse to create a spatial superposition, followed by a $\pi$ pulse to redirect the atomic trajectories, and finally another $\pi/2$ pulse to interfere both branches.
The pulses are separated by a time interval $T$.
For the Bragg-Mach-Zehnder scheme we calculate the phase via a perturbative formalism~\cite{Ufrecht2019,Ufrecht2020b}:
We split the Hamiltonian into an unperturbed part $\hat{H}^{(\sigma)}_0$, defined by the first line of Eq.~\eqref{eq:Hamiltonian}, and a perturbation $\hat{\mathcal{H}}^{(\sigma)}$ given by the second line.
Moreover, we consider the classical trajectories generated by a classical counterpart of $\hat{H}^{(\sigma)}_0$.
These unperturbed trajectories are inserted into the perturbing classical counterpart of $\hat{\mathcal{H}}^{(\sigma)}$ and integrated along the upper and the lower branch.
For unperturbed interferometers closed in phase space this procedure leads to a phase
\begin{align}
\label{eq:general_phase}
    \varphi=\varphi_0-\frac{1}{\hbar}\int\text{d}t~\left(\mathcal{H}^{(u)}-\mathcal{H}^{(l)}\right)+\varphi_\text{FSL}.
\end{align}
Here, $\varphi_0=-kgT^2$ arises from the unperturbed Hamiltonian $\hat{H}^{(\sigma)}_0$~\cite{Kleinert2015}.
Cross terms between perturbations are of higher order and are, consequently, neglected.
Since we are interested in relativistic effects due to light propagation, we also include~\cite{Dimopoulos2008,Tan2016,Tan2017} the finite-speed-of-light contribution $\varphi_\text{FSL}$.
This additional term $\varphi_\text{FSL}=-3 k g T^2 v_T/c$ depends on the velocity $v_T=v_0-g T+\hbar k/m$ on the upper branch at the central pulse, with initial velocity $v_0$ at the first pulse.
Although $\varphi_\text{FSL}$ has been derived before~\cite{Dimopoulos2008,Tan2016,Tan2017}, we analyze its effect in different situations.

\subsection{Gravitational effects including the dilaton}
In this section we analyze the effect of gravity including the dilaton field on atom interferometry both via light propagation and the coupling of the atomic mass to the dilaton.
To highlight the gravitational contributions, we set $\varrho_0=0$, i.\,e., we consider only the influence of the gravitational source mass on the dilaton field and neglect the background oscillation.
To lowest order in all perturbative parameters we obtain the phase
\begin{align}
\label{eq:SinglePhase}
	\begin{split}
		-\frac{\varphi}{k g T^2}=&1+\beta+3\frac{v_T}{c}+ \frac{v_0v_T}{c^2}- \frac{g z_T}{c^2}\\
		&- \frac{g T}{c^2} \left( v_0+ \frac{\hbar k}{2 m} - g T\right)+ \frac{g^2T^2}{4c^2}
	\end{split}
\end{align}
apart from a trivial laser contribution.
Here, we introduced the atom's initial position $z_0$, as well as the atomic position $z_T=z_0+v_0T-gT^2/2+\hbar k T/m$ on the upper branch during the central pulse.
The first term represents the conventional gravimeter phase~\cite{Kasevich1991,Kleinert2015}.
The second term corresponds to the leading dilaton violation of EEP~\cite{Fray2004,Bonnin2013,Schlippert2014,Zhang2018,Asenbam2020}.
The third term stems from finite speed of light~\cite{Dimopoulos2008,Tan2016,Tan2017}.
All remaining terms result from the modified wave vector.
They resemble phases caused by gravity gradients~\cite{Kleinert2015}, since the perturbative potential in Eq.~\eqref{eq:kick-potential} is quadratic in the atom's position.
In principle, all additional contributions in Eq.~\eqref{eq:SinglePhase} limit the sensitivity of gravimeters, but are usually negligibly small compared to other deleterious effects.
However, in the following we discuss their effect in differential measurements where other noise sources are suppressed.

\subsubsection{Atom-interferometric gradiometry}
Atom-interferometric gradiometers~\cite{Snadden1998,McGuirk2002,Abe2021} can be built from two identical interferometers, each with individual (but possibly phase-locked) lasers, vertically separated by a length $\ell$.
We assign an index $j=1,2$ to the upper and lower interferometer, which allows us to infer the differential phase $\delta\varphi=\varphi_1-\varphi_2$ between both signals.
Each phase is associated with a local linear acceleration $g_j$, with mean acceleration $g=(g_1+g_2)/2$ and difference $\delta g=g_1-g_2$.
They capture the change of the gravitational field due to higher gravitational multipoles between the atom interferometers and correspond to two different expansion points of the metric.
However, the treatment neglects local gravity gradients on the scale of the extension of the individual interferometer~\cite{Roura2014,DAmico2017,Ufrecht2021}.
Since effects from the modified wave vector scale with $c^{-2}$, we also neglect its cross terms with $\delta g$.
If we prepare equal initial velocities, we find the differential phase
\begin{align}
	\begin{split}
		\frac{\delta\varphi}{kgT^2}=-\frac{\delta g}{g}\left(1+\beta+3\frac{v_T-gT}{c}\right)+\frac{g\ell}{c^2}
	\end{split}
\end{align}
between both interferometers.
The contribution from the modified wave vector grows with increasing spatial separation and is of order $g\ell/c^2\cong10^{-13}$ for planned separations of up to $10^3\,$m for Earth-based setups~\cite{Abe2021}.
Even though such devices are mainly limited by gravity-gradient noise, this phase contribution has to be taken into account for a thorough analysis.
At the same time, it offers an atom-interferometric verification of the influence of gravity on light, so far primarily observed in an astronomical or cosmological context.
Similarly, finite speed of light sets limits on the accuracy of gradiometers and crucially depends on the velocity of the atoms at the central pulse.

\subsubsection{EEP tests with atom interferometry}
Atom-interferometric tests of EEP~\cite{Fray2004,Bonnin2013,Schlippert2014,Zhang2018,Asenbam2020,Roura2020,Roura2020b,Bothwell2021,Ufrecht2020,DiPumpo2021} involve differential phases between two species or atomic levels, labeled by the index $j=a,b$.
For two masses $m_a$ and $m_b$ we calculate the differential phase $\theta_k=\varphi_a/(|k_a| g T^2)-\varphi_b/(|k_b| g T^2)$, where $m_j=m+\lambda_j\Delta m/2$ with $\lambda_b=1$ and $\lambda_a=-1$.
Here, $m = (m_a+m_b)/2$ is the mean mass.
Similarly, each atomic component is addressed by a different laser and therefore experiences a different momentum transfer $\hbar k_j = \hbar k+\lambda_j\hbar \Delta k/2$.
We also introduce different violation parameters $\beta_j$, as well as different initial values for position and velocity.
For $k_b,k_a>0$ we obtain
\begin{align}
\label{eq:DiffPhase}
	\begin{split}
		\theta_k=&\Delta\beta+3\frac{\Delta v_0}{c}-\frac{g}{c^2}\left(\Delta z_0+3\Delta v_0T\right)+2\frac{v_0\Delta v_0}{c^2} \\
		&+ \chi  \frac{v_\text{r}}{c}\left(3-\frac{3g T}{2c}+ \frac{v_0}{c} \right)\left(\frac{\Delta k}{k}-\frac{\Omega}{\omega_C}\right)\\
		&+\chi\frac{v_\text{r}\Delta v_0}{c^2}\left(1-\frac{\Delta k}{4k}\frac{\Omega}{\omega_C}\right)
	\end{split}
\end{align}
with the violation parameter $\Delta\beta=\beta_b-\beta_a$, which can be used to parametrize UFF tests~\cite{Fray2004,Bonnin2013,Schlippert2014,Zhang2018,Asenbam2020}.
Here, we introduce the average recoil velocity $v_\text{r} = \hbar k /m$ and different initial velocities $v_0+\lambda_j\Delta v_0/2$ and positions $z_0+\lambda_j\Delta z_0$.
The parameter $\chi=\big[1-\Omega^2/(2 \omega_C)^2\big]^{-1}$ quantifies the magnitude of the mass difference, where we defined $\Omega=\Delta m c^2/\hbar$ and the frequency $\omega_C=m c^2/\hbar$.

Quantum clock interferometry~\cite{Sinha2011,Zych2011,Rosi2017,Loriani2019,Ufrecht2020,Roura2020,Roura2020b,DiPumpo2021} is based on a superposition of two different internal states.
Even though their eigenenergies are associated with different masses~\cite{Lammerzahl1995,[][ and references therein.]Pikovski2017,Sonnleitner2018,Schwartz2019} through the relativistic mass-energy relation, the factor $\Omega/\omega_C\ll1$ acts perturbatively.
Such interferometers are often operated with magic Bragg diffraction~\cite{Katori2003}, which implies $\Delta k=0$.
Similarly, the differences $\Delta v_0$ and $\Delta z_0$ for two internal states are strongly perturbative and can be neglected when divided by the speed of light.
As a consequence, only the dilaton-dependent term $\Delta\beta$ is relevant for EEP tests via quantum clock interferometry.

For different atomic species their mass difference is of the order of the mean mass so that the arguments for quantum clock interferometry do not apply.
However, when performing conventional UFF tests with distinct atomic species~\cite{Fray2004,Bonnin2013,Schlippert2014,Asenbam2020} the momentum kick $k_j$ is reversed~\cite{McGuirk2002} for both species after each experimental run.
This way, noise and other deleterious effects are removed from the signal.
Hence, we find the two-fold differential phase
\begin{align}
\label{eq:TwoFoldPhase}
	\begin{split}
		\frac{\theta_k-\theta_{-k}}{2}=\Delta\beta+3\frac{\Delta v_0}{c}+2\frac{v_0\Delta v_0}{c^2}-\frac{g\Delta z_0}{c^2}-3\frac{g\Delta v_0T}{c^2}
	\end{split}
\end{align}
leading to the cancellation of all effects linear in $k_j$.
Apart from the UFF violation parameter, only effects from different initial positions and velocities survive this $k$-reversal technique.
These remaining terms are dominated by the finite-speed-of-light effect $3\Delta v_0/c$.
The estimate for already performed UFF tests~\cite{Bonnin2013} was $\Delta v_0/c\cong 2\cdot10^{-11}$, which is close to the uncertainty of planned experiments~\cite{Schlippert2020}.
As such, the effect has to be subtracted for the analysis of the test.
To this end, the error $\delta(\Delta v_0)$ caused by the uncertainty of the differential initial velocity remains~\cite{Nobili2016}.
Assuming~\cite{Loriani2020} $1\,$\textmu m/s leads to $\delta(\Delta v_0)/c\cong3\cdot10^{-15}$.
As a consequence, the remaining effect from finite speed of light in UFF tests with two species can be removed from the signal up to a precision of $10^{-15}$ due to good control over the initial velocities.
The other terms in Eq.~\eqref{eq:TwoFoldPhase} proportional to $\Delta v_0$ are further suppressed by the inverse speed of light.
They can be neglected for state-of-the-art and near-future schemes.
Similarly, the term proportional to $\Delta z_0$ is also of no relevance for UFF tests so far.
Finally, we see that only the atom's propagation in the dilaton field induces phases sensitive to UFF violations.
This observation can be tracked back to the fact that the dilaton only modifies the Rabi frequency of the diffracting pulse but not the momentum transfer.
Consequently, the propagation of light in dilaton gravity does not contribute to these violations.

\subsection{Effects of oscillating dilaton field}
In this section, we consider the coupling of the time-dependent part of the dilaton field, not caused by the source mass, to an atom interferometer, as for example used as a model in the context of dark-matter detection~\cite{Geraci2016}.
Similar to gradiometry, the detection scheme~\cite{Arvanitaki2018,ElNeaj2020,Badurina2021} is based on differential phases $\delta\varphi=\varphi_1-\varphi_2$ between two identical atom interferometers operated at different locations.
For example, in proposed space-based gravitational-wave~\cite{Dimopoulos2009,Hogan2016} and dark-matter detection schemes~\cite{ElNeaj2020} two atom interferometers are placed at distances kilometers apart from each other.
Due to microgravity, we have $g=0$.
This choice naturally leads to a cancellation of all finite-speed-of-light effects that arise within each interferometer, as wells as all effects from the modified wave vector, since they are proportional to the gravitational acceleration.
We calculate the phase of one atom interferometer similar to Eq.~\eqref{eq:SinglePhase} but with $g=0$, and solely include the plane-wave part of the dilaton field.
However, the interferometers interact with the light pulses at locations separated by $\ell$, which implies an offset $\ell/c$ between the start of the interferometers.
By taking the different initial times into account and assuming the same initial velocity $v_0$, we find the differential phase
\begin{align}
	\begin{split}
		\frac{\delta\varphi}{(ckT)^2}&=-2\varrho_0\frac{k_\varrho}{k}
		\cos{\left(\omega_\varrho T -k_\varrho \bar z_T + \frac{\omega_\varrho \ell}{2c}+\phi_\varrho\right)} \\
		&\times \sin{\left( \frac{\omega_\varrho \ell}{2c} \left[1-\frac{ck_\varrho}{\omega_\varrho}\right]\right)}
		\operatorname{sinc}{\left(\frac{\omega_\varrho T}{2}\left[1-\frac{v_0 k_\varrho}{\omega_\varrho}\right]\right)}  \\
		&\times\operatorname{sinc}{\left(\frac{\omega_\varrho T}{2}\left[1-\frac{v_T k_\varrho}{\omega_\varrho}\right]\right)}
	\end{split}
\end{align}
with average position $\bar z_T=\ell+v_0 T+\hbar k T/(2m)$ and velocity $v_T=v_0+\hbar k/m$ on the upper branch at the central pulse of each interferometer.
Such schemes measure the different couplings of the dilaton to the atom's mass between the two interferometers.
These different couplings are caused by the oscillations of the background field.
Since the initial phase $\phi_\varrho$ of the dilaton field is unknown, we find the amplitude of the fluctuations induced by the dilaton field and measured by a continuous operation of the detector from $\varphi_\text{SA}= \left(\int_0^{2\pi}{\mathrm{d}\phi_\varrho~\delta\varphi^2/\pi}\right)^{1/2}$.
It corresponds to the standard deviation of the phase signal.
The amplitude takes the form
\begin{align}
	\begin{split}
		\frac{\varphi_\text{SA}}{(ckT)^2}&=2\varrho_0\frac{k_\varrho}{k}
		\sin{\left( \frac{\omega_\varrho \ell}{2c} \left[1-\frac{ck_\varrho}{\omega_\varrho}\right]\right)} \\
		&\times\operatorname{sinc}{\left(\frac{\omega_\varrho T}{2}\left[1-\frac{v_0 k_\varrho}{\omega_\varrho}\right]\right)}\operatorname{sinc}{\left(\frac{\omega_\varrho T}{2}\left[1-\frac{v_T k_\varrho}{\omega_\varrho}\right]\right)},
	\end{split}
\end{align}
which shows that the influence of the oscillating background can indeed be resolved in such differential setups.
We emphasize that for ceasing dilaton mass $m_\varrho$, i.e., $\omega_\varrho = c k_\varrho$, the signal amplitude vanishes.
Note that the assumption of the dilaton's Compton wave length being much larger than the extension of the experiment (see Appendix~\ref{sec:App}) is not necessary for such spaceborne schemes, since the gravitational part of the dilaton field vanishes here.
Similarly, for vanishing dilaton recoil $\hbar k_\varrho$, the limit usually discussed in the context of dark-matter detection with atom interferometers~\cite{Geraci2016,Arvanitaki2018,ElNeaj2020,Badurina2021}, the signal amplitude also vanishes.
As such, our result differs from these previous ones, as we perform only first-order perturbation theory but include also the dilaton mass and the dilaton recoil in our Hamiltonian from Eq.~\eqref{eq:Hamiltonian}.
Although the laser propagates through the dilaton field, this propagation does not imprint dilaton-dependent terms on the signal.
In contrast, similar to the Earth-based schemes discussed before, it is the atom's mass which probes the oscillating background imprinting the phase.

\section{Discussion}
We derived dilaton-modified Maxwell equations from a first-principle Lagrangian approach, and solved them with a geometrical-optics ansatz.
The resulting phase of the electromagnetic field is not influenced by the dilaton to lowest order, in contrast to the amplitude which experiences a dilaton-dependent modification.
Nevertheless, gravity alters the wave vector of the electromagnetic field.
Consequently, no dilaton effects are imprinted by the light's phase in atom-optical experiments, although the momentum transfer on the atom is modified by gravity.
However, the dilaton couples to the mass-energy of the atom and, therefore, affects the time evolution of the atomic structure and center-of-mass motion.

To illustrate our results, we analyzed two scenarios for a light-pulse Mach-Zehnder atom interferometer:
a dilaton field solely sourced by Earth's mass and an oscillating background field of cosmic origin.
In the first case, we showed that for gradiometers the effects from finite speed of light and the gravitationally modified wave vector are the dominant contributions.
For EEP tests, however, only the UFF violation parameter survives for quantum clock experiments performed with a superposition of internal states.
Differential effects are negligible because the mass-energy difference of two such states is small and no colocation issues arise in the state preparation.
Contrarily, for ambitious UFF tests with different species and a $k$-reversal technique, additional effects from finite speed of light can become relevant.
We discussed the detection of dark matter in spaceborne experiments by probing an oscillating dilaton field at different locations in spacetime with two atom interferometers.
Already a spatial dependence of the dilaton leads to measurable effects, a fact not accounted for in most studies of atom-interferometric dark-matter detectors.

Hence, this article provides a discussion of the leading-order propagation of all constituents relevant for light-pulse atom interferometers in gravity and dilaton fields, i.\,e., the propagation of light and matter.
While the propagation of matter gives rise to dominant effects, corrections from the propagation of light in gravity has to be taken into account for future high-precision experiments.
Thus, our results constitute a framework for the analysis of atomic experiments where the propagation of light plays a crucial role, such as gravitational wave or dark matter detectors.
Consequently, they can be used to constrain parameters that describe extensions of the Standard Model or general relativity, as exemplified by the dilaton field.
The potential of atom interferometry for fundamental physics can be highlighted by future studies of different geometries beyond the examples discussed in our article.

\begin{acknowledgments}
We are grateful to W. P. Schleich for his stimulating input and continuing support.
We also thank W. G. Unruh, as well as the QUANTUS and INTENTAS teams for fruitful and interesting discussions.
The projects ``Metrology with interfering Unruh-DeWitt detectors'' (MIUnD) and ``Building composite particles from quantum field theory on dilaton gravity'' (BOnD) are funded by the Carl Zeiss Foundation (Carl-Zeiss-Stiftung).
The work of IQ\textsuperscript{ST} is financially supported by the Ministry of Science, Research and Art Baden-W\"urttemberg (Ministerium f\"ur Wissenschaft, Forschung und Kunst Baden-W\"urttemberg).
The QUANTUS and INTENTAS projects are supported by the German Aerospace Center (Deutsches Zentrum f\"ur Luft- und Raumfahrt, DLR) with funds provided by the Federal Ministry for Economic Affairs and Climate Action (Bundesministerium f\"ur Wirtschaft und Klimaschutz, BMWK) due to an enactment of the German Bundestag under Grants No. 50WM1956 (QUANTUS V), No. 50WM2250D-2250E (QUANTUS+), as well as No. 50WM2177-2178 (INTENTAS).
E.G. thanks the German Research Foundation (Deutsche Forschungsgemeinschaft, DFG) for a Mercator Fellowship within CRC 1227 (DQ-mat).
\end{acknowledgments}

redpajama_set_name: RedPajamaArXiv


text:
Q: How to boot computer without acpi=off I recently bought an gaming laptop (the Gigabyte Sabre 15) with an Nvidia geforce gtx 1050. I had trouble with the graphic card during the installation of ubuntu and I had to boot with acpi=off.
Now everything is installed (including Nvidia drivers which was not as easy as usual) and i don't want my computer to boot with acpi=off anymore because it causes trouble with my keyboard and touchpad. I can disable it at start up by going into the grub and then by erasing "acpi=off" in the boot parameter, but then it works just once. And i don't want to do it at every boot.
Someone could give me a permanent solution? Thank you!

A: To permanently remove acpi=offfrom the GRUB options, you have to edit the file /etc/default/grub.
You'll find a line like
GRUB_CMDLINE_LINUX_DEFAULT="quiet splash acpi=off"

or similar (the important part is GRUB_CMDLINE_LINUX_DEFAULT, and obviously there should be acpi=off).
Just remove the acpi=off part (GRUB_CMDLINE_LINUX_DEFAULT="quiet splash"), save, exit and run
sudo update-grub

redpajama_set_name: RedPajamaStackExchange


What Does the New Moon on December 7 Have in Store for You?
Mercury elongation, Geminids meteor shower, Ursids meteor shower, and December solstice, are only a few amongst many Astronomical events taking place in December 2018. We may not realize but there's a lot happening out up there in the endless dark stretches. And let's face it, either it's a meteor shower, stars crashing into each other, or regular planetary retrogrades, these cosmological events have a tremendous impact on our daily lives. Now here, we may not talk about one of such spectacular event but we definitely have managed to crack up your mood for some Astrology stuff.
Astrologers consider new Moon a good omen which can be well attributed to the fact that it represents the brightest day of the lunar cycle and occurs after constantly changing phases between darkness and light. This whole idea seems to have a certain philosophical bent to it but even scientifically and astronomically, the day of New Moon kind of acts as a catalyst for the zodiacs. And since December 2018's new Moon is the first since Jupiter moved into Sagittarius, you can expect it to be extra special in terms of enhanced capabilities, fruitful opportunities, and luck.
You see, Sagittarius is the planet that is believed to be the significator of travel, personal growth, and excitement. It is considered a fearless zodiac sign. One that is capable of discovering new limits through its need to understand the real purpose of life. So this moon is going to endow upon you the capabilities to expand your horizon as an individual at home, at work, and at every significant aspect of life that ensures you moving forward. You'd be able to unlock your potential!
Read More: Sagittarius Daily Horoscope!
Two planetary bodies namely Mars and Pluto are merging into each other this month which sends you into an overdrive to realizing newer paths to follow. Something that you normally won't do. Mars represents our fearless and active side whereas Neptune connects the inner knowledge to intuition. Interesting mix of planets and qualities there as this New Moon inspires you to decode the mysteries of the unknown and foresee the results.
This can be understood by a simple interpretation of this scenario which states you'd be able to follow your passion without hesitation. So if you are looking to switch your field of study all of a sudden, then December could be the month for you. Or it could make you go down the spiritual path in a trice. By the end of it all, you'd be curled up with one of your passion or something that you always wanted to do.
This #NewMoon will also help you realize that your experience on Earth is measured by the variety of places you have explored. This exploration may not have a literal significance in your context as the journey you would be embarking upon would be more about discovering the different sides of your personality.
Different natal charts have a different impact by the new Moon on them but one thing is going to be sure – karma and fate prevailing through life. This is mainly because Mercury, a planet that rules mind, perspective, and one's ability to perceive reality is slowly moving into Scorpio. The New Moon will be at a point within the chart that lights up the area representing the so-called cause and effect zone. Plus there is a pretty strong chance that you might experience a troubling time in your life which we think could well be the result of your actions and part of your destiny.
Read More: Is a Zodiac Compatibility a Real Thing in Relationship?
The North Node during this event falls on the very emotional, nurturing and sensitive Cancer. This refers to a comfortable home environment. However, this doesn't necessarily mean things are going to stay same forever, you have to work hard. For that, Mercury will guide you onto a greater life path where you'd be able to restore peace in your life.
Well, there'll be a lot of things happening in your life this month so here's wishing you all the luck in the world and may this New Moon brightens your world with happiness and success.
And since it's the holiday season, don't miss out on our fabulous festival articles this Thanksgiving, Halloween, and Christmas.


text:
Search results for 'world war II'
SAS publishes top secret World War II diary
Kept secret for 65 years, the SAS publishes a diary charting daring missions carried out during its earliest days in World War II, including an operation to capture German commander Erwin Rommel.
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Japan's Prime Minister says the earthquake, tsunami and nuclear incidents are "the biggest crisis for Japan since World War II." Channel 4 News speaks to a woman who cannot reach her family.
Channel Island's World War II forgotten heroes revealed
Documents outlining the bravery of Channel Islanders who resisted the Nazis in World War Two have been discovered after almost 50 years. Channel 4 News talks to relatives of those in the resistance.
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The Polish Government has found itself accused of a 'Cultural Purge' after the boss of the country's World War II Museum was sacked.
Establish a 'truth and reconciliation commission' to heal Windrush wounds, Barbados High Commissioner warns
In a heartfelt and searing goodbye letter to Britain, the departing Barbados High Commissioner has told Channel 4 News that the UK should establish a "truth and reconciliation commission" to deal with the fall out from the Windrush scandal.
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Thousands of passengers had their flights and trains cancelled today – after a 500kg world war two bomb was found in the river Thames. London City airport was forced to close and families living within an exclusion zone have been evacuated from their homes as experts from the Royal Navy and police try to remove…
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A controlled explosion on a second world war bomb is carried out, after it was found near Wembley Stadium in north-west London.
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More than 50 million people were forced to leave their homes last year due to war or persecution, the highest number since the second world war, says the UN refugee agency.
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Germany and France have warned Russia that it will face "appropriate consequences" if the 25 May election in Ukraine does not go ahead as planned.
Anthony Scaramucci: Trump's comments 'reminiscent of what my grandparents had to hear'
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New European chief open to another Brexit delay

redpajama_set_name: RedPajamaCommonCrawl


text:
What are the 5 sources of law?
Ben Davis May 19, 2020
What are the two sources of criminal law?
What are the four sources of criminal and civil laws?
What are the major sources of law?
What are the 5 sources of law in the United States?
What is state law and example?
Why are state laws different?
What are some good ideas for laws?
Can a federal law be changed?
Why was a federal law necessary?
What are examples of local laws?
How can a local law be changed?
What is another name for local law?
The primary sources of law in the United States are the United States Constitution, state constitutions, federal and state statutes, common law, case law, and administrative law.
Section 3.1: Sources of Criminal Law
The Common Law.
Constitutions.
Statutory Law.
Administrative Law.
Court Cases.
These four sources of law are the United States Constitution, federal and state statutes, administrative regulations, and case law.
Primary sources of law are constitutions, statutes, regulations, and cases. Lawmaking powers are divided among three branches of government: executive; legislative; and judicial. These three branches of government, whether federal or state, create primary sources of law.
In the United States, the law is derived from five sources: constitutional law, statutory law, treaties, administrative regulations, and the common law (which includes case law).
For example, laws on commerce, bankruptcy or taxation are made at the federal level. State and local governments pass laws about property, divorce, custody, and other matters that really don't affect anyone outside of that state.
There are actually two different sets of laws; federal laws and state laws. Constitutional law permits each state to create and enforce additional laws for their state. Each state is considered sovereign and has the power to create laws as needed. Each state is considered unique with its own characteristics.
10 Ideas that should be laws in the United States
Yellow #5 should be banned.
Limit house holds to one car.
Fast food should be illegal.
Make schools start at 5 am.
Make Tobacco Illegal.
Energy drinks should be banned.
Gambling should be banned.
Make lunches free at schools.
Laws must be enacted and implemented consistently with the U.S. Constitution. Laws can be changed or amended only when Congress enacts, and the President signs, a later law.
Laws protect our general safety, and ensure our rights as citizens against abuses by other people, by organizations, and by the government itself. We have laws to help provide for our general safety.
10 Local Laws That May Be Doing More Harm Than Good
Nuisance Laws.
Jaywalking Laws.
Fines for Minor Infractions.
Privatizing Water.
Occupancy Standards for Rental Housing.
Criminalizing Food Sharing.
Tobacco "PUP" Laws.
School Discipline Policies.
If you are going to change a local law, you need support from someone in the city government. If you don't want to approach the mayor directly, choose the council member from your district or one you think will be sympathetic to your cause. Meet with your chosen lawmaker.
What is another word for local law?
bylaw
decree act
ordinance command
edict canon
dictate commandment
Category: Sociology
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Thanks for that but I already have it install. I had to update meson (sudo pip3 install meson) from 3.7 > 4.8 need at lease 4.7 then I installed ninja git clone git://github.com/ninja-build/ninja.git && cd ninja v1,8,2.
I quite like installing with meson this is not the only program that I install with meson.
Was just trying to keep the repository update to date.. Hopeful I am not the only one that uses this great little program.
Arch will always keep programs like this update to date as a lot of users run DMs like i3 and mpd is a gem on i3 as it is vim based.. or any other DM. and is non GUI.
It is people like you that make Debian base systems so much more FUN to use. Thank You So Much for All your time...and all the Coders. Also Thanks for the repology.org link.
We also have Meson 0.48.1 in the test repo--I had to use it to build the new mpd.
Lmao I'm aloud to have some Fun too .


text:
PAST CHAMPIONS CONFIRMED FOR 2015 CANADIAN PACIFIC WOMEN'S OPEN
Defending champion So Yeon Ryu, Brittany Lincicome, Michelle Wie, Suzann Pettersen, Katherine Hull and Cristie Kerr will join Lydia Ko who returns to The Vancouver Golf Club for the first time since historic victory in 2012
17-year old Brooke Henderson of Smiths Falls, Ont. granted tournament exemption to compete in Canada's National Women's Open for the fourth time
Support BC Children's Hospital and Pediatric Heart Health through the CP Has Heart program; Free Admission for juniors aged 17 & under
Coquitlam, B.C. (Golf Canada) – Golf Canada in partnership with Canadian Pacific (CP) have announced that defending champion So Yeon Ryu will headline a list of seven past champions who have confirmed their intention to challenge for the US$2.25 million purse at the 2015 Canadian Pacific Women's Open.
Currently ranked No. 7 on the Rolex World Ranking, Ryu played near flawless golf last August at the London Hunt and Country Club to capture the inaugural Canadian Pacific Women's Open. A three-time winner on the LPGA Tour, Ryu's 23-under tournament total in 2014 set a new event scoring record in relation to par.
Also confirming her intention to compete for Canada's National Women's Open title will be two-time champion Lydia Ko (2012 & 2013), the current World No. 2 who made history at The Vancouver Golf Club in 2012 when she captured her first LPGA Tour victory as a 15-year old amateur.
In addition to Ryu (2014) and Ko (2012 & 2013), other past champions set to compete include World No. 5 Suzann Pettersen (2009), World No. 8 Brittany Lincicome (2011), World No. 12 Cristie Kerr (2006), World No. 14 Michelle Wie (2010) and Katherine Hull (2008).
"We're two months away from the Canadian Pacific Women's Open and we are very pleased with how our field is coming together," said Canadian Pacific Women's Open Tournament Director, Brent McLaughlin. "We are fortunate to have a terrific history of champions and I know it will be especially exciting for Vancouver golf fans to welcome Lydia Ko back to The Vancouver Golf Club for the first time since her amazing win in 2012."
Golf Canada also confirmed that 17-year old Brooke Henderson of Smiths Falls, Ont. has been granted an exemption to compete in the Canadian Pacific Women's Open. Henderson, a member of Golf Canada's Young Pro Squad and currently the No. 51 ranked player in the world, will be making her fourth consecutive appearance in Canada's National Women's Open Championship. In her first year as a professional, the former World No. 1 ranked amateur has amassed $317,470 in LPGA earnings including $132,725 for her tie for 5th finish this past weekend at the KPMG Women's PGA Championship.
"Brooke has had an outstanding start to her pro career and it comes as no surprise that she has earned an exemption to compete in Canada's National Women's Open for the fourth time," said McLaughlin. "She's a special player and a terrific ambassador for Canadian golf and I'm sure she'll be fan favourite once again at The Vancouver Golf Club."
Henderson will lead a Canadian contingent that also includes four-time LPGA Tour winner and Canadian Pacific ambassador Lorie Kane of Charlottetown as well as LPGA Tour players Alena Sharp of Hamilton, Ont. Sue Kim of Langley, B.C. and Rebecca Lee-Bentham of Toronto.
Additional Canadian and international exemptions into the National Women's Open Championship will be announced in the coming weeks. A field of 156 competitors will vie for the US$2.25 million purse when the CP Women's Open makes its return to The Vancouver Golf Club.
The 2015 Canadian Pacific Women's Open is proud to support BC Children's Hospital as the 2015 charity beneficiary of this year's event.
Funds raised this year will be dedicated to the pediatric cardiology research program.
As part of its community investment program CP Has Heart, CP is matching all online donations through www.bcchf.ca/cphasheart until August 23. Fan and player favourite, Birdies for Heart, also returns this year with CP committed to donating $5,000 for every birdie made on the 17th hole. In 2014, Birdies for Heart raised more than $320,000 for charity during tournament week.
Free Admission for Juniors…
Golf Canada and CP are proud to offer free admission to the Canadian Pacific Women's Open to any spectator aged 17 and under. In addition to free admission for juniors, parents can take advantage of discounted tickets by visiting www.cpwomensopen.com/tickets and using promo code "junior".
Juniors – 17 & Under Free
Early Week (Mon-Wed) $10 ($15 @ the gate)
Anyday Grounds (Thurs-Sun) $30 ($40 @ the gate)
Weekly (Mon-Sun) $75 ($100 @ the gate)
Clubhouse Badge Single $175
Clubhouse Badge Twosome $300
Clubhouse Badge Foursome $550
First conducted in 1973, Canada's National Women's Open Championship has allowed the brightest stars of the LPGA Tour to shine on Canadian soil and inspire the nation's next generation of female golfers.
Additional information regarding tickets, volunteer opportunities and corporate hospitality for the 2015 or 2016 Canadian Pacific Women's Open can be found at www.cpwomensopen.com.
ABOUT THE 2015 CANADIAN PACIFIC WOMEN'S OPEN
The stars of the LPGA Tour will challenge for the Canadian Pacific Women's Open from August 17-23 at The Vancouver Golf Club in Coquitlam, B.C. The Canadian Pacific Women's Open, Canada's National Women's Open Golf Championship, is proudly sponsored by Canadian Pacific, RBC, WestJet, Molson Canadian 67, TaylorMade adidas Golf, TY KU, Santa Carolina Wines, Coca-Cola, Executive Hotels & Resorts, Ford Motor Company and CVS Controls LTD. For information on volunteer opportunities, tickets or corporate hospitality, visit www.CPwomensopen.com, or call 1-866-571-5742.
ABOUT CP HAS HEART
At CP, we know that a railroad may serve as the arteries of a nation, but at its heart is community. That's why, through CP Has Heart, we've already committed more than $5 million dollars to help improve the heart health of men, women and children across North America. And along the way, we're showing heart whenever we can. Find out more on www.cpr.ca or @CPhasHeart.
ABOUT CANADIAN PACIFIC
Canadian Pacific (TSX:CP)(NYSE:CP) is a transcontinental railway in Canada and the United States with direct links to eight major ports, including Vancouver and Montreal, providing North American customers a competitive rail service with access to key markets in every corner of the globe. CP is growing with its customers, offering a suite of freight transportation services, logistics solutions and supply chain expertise. Visit www.cpr.ca to see the rail advantages of Canadian Pacific.
GOLF CANADA – LOVE THE GAME. GROW THE GAME.
Golf Canada is the National Sports Organization and governing body for golf in Canada representing close to 310,000 golfers at more than 1,400 member clubs across the country. A proud member of the Canadian Olympic Committee, Golf Canada's mission is to grow participation, excellence and passion in the sport while upholding the integrity and traditions of the game. By investing in the growth of the sport and introducing more participants of all ages to the game, our goal is to be relevant to and respected by all Canadian golf enthusiasts from coast to coast. For more information about what Golf Canada is doing to support golf in your community, visit www.golfcanada.ca.
Dan Pino
(p) 1-800-263-0009 ext. 406
(e) dpino@golfcanada.ca
Jeremy Berry
Director Media Relations
(p) (403)319-6227
(e) jeremy_berry@cpr.ca


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See how easy it is to turn your backyard into your private year round oasis.
We'll give you a free estimate, design assistance and in a few months your oasis will be your family's favorite entertainment and activity area.
All swimming pool enclosures made in the USA, we install anywhere in the United States.
Swimming pool enclosures require special attention to engineering, load requirements, ventilation and other unique issues.
So you've looked at the photos, read about the many benefits and now you're ready to find out the price of a pool enclosure.


In order to perform data integration operations, you need to create a connection first. You can create a connection on the Connections page.
Read more about available connections.
Step 1. To create a new connection, go to the Connections page (left menu) and click the + button. Then click the corresponding connection type in the opened box.
To quickly find the corresponding type, you can enter all or a part of the name in the search box. Then, only the types with the entered string in their names will be displayed. To filter connections by category, click the corresponding connection category from the list to the left of the connection-type grid.
Step 2. After the connection type has been selected, continue by entering the connection parameters.
Always encrypt credentials using a long encryption key and a strong encryption algorithm.
Never send credentials to a web browser.
Step 3. After a connection has been created, you can test it by clicking the Test Connection button.
the Test Connection button is not visible for some types of connections, such as for HTTP.
Step 4. After a connection has been tested, you can save it by clicking the Save button.
All saved connections are displayed in a grid on the Connections page and can be quickly filtered by name and type. Connections can be modified, duplicated, or deleted from within the grid.
when the connection is getting duplicated the password associated with the connection is getting reset.


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Q: Why $\log\mathrm{det}(A (A^{-1}B)^{1/2}) = \log\mathrm{det}(A^{1/2}B^{1/2})$
$A,B$ are positive definite matrices.
  Show
  $$\log\mathrm{det}\left( A^{1/2} (A^{−1/2} B A^{−1/2})^{1/2} A^{1/2} \right) = \log\mathrm{det}(A^{1/2}B^{1/2}) $$

I have known :
$$ A^{1/2} (A^{−1/2} B A^{−1/2})^{1/2} A^{1/2} = A (A^{-1}B)^{1/2} $$
But I can't get
$$\log\mathrm{det}(A (A^{-1}B)^{1/2}) = \log\mathrm{det}(A^{1/2}B^{1/2})$$
I hope someone will help me. Thank you.

A: Note that $\det(AB) = \det(A)\det(B)$ and $\det(A^{1/2}) = \sqrt{\det(A)}$. Use these to pull apart the determinants into products and powers of real numbers, then check if they're equal.


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You can make a mind map with no hands in just three steps on an iPhone.
1. Outline the text of your mind map in Drafts.
To get going, use Siri to record what will be your first node.
To get to a second node, simply say, "New line, new line" and say what your next node will be.
If you want to do sub-nodes (i.e., "children") after you have dictated your main/parent node, say, "New line," and then have Siri indent your sub-node with the "tab key" command. Then dictate that sub-node or child.
You can add more parent, child, and sibling topics similarly.
2. Run your "Open in…" action in Drafts.
3. View your mind map in MindNode.
Because of MindNode's iCloud-enabled sync setup, you can now view (and modify) your mind map in iOS or OSX platforms.
The above is an adaptation/re-posting of a previous post on voice dictating a mind map. That post used the app iThoughts, but I learned shortly after posting that even though MindNode doesn't have the x-callback-url support that iThoughts does, Drafts's "Open in…" feature makes the same process possible with just one extra tap. Rad.


According to the Census Bureau's American Community Survey, women comprise 48 percent of the U.S. workforce — but just 24 percent of workers in STEM fields.
These numbers stem from pipeline issues, personal choices, and biases — where women who are looking to specialize in subjects ranging from astrophysics to marine microbiology are being edged out.
EXPLO is looking to change all of that.
Our Bioengineering for Girls program (for students entering grades 9-11) welcomes young women into college labs under the instruction of Professor Laura Ekstrom, and connects them with professionals and researchers from around the U.S. who introduce them to the many opportunities and possibilities in the field. They leave the program with an introduction to bioengineering research, an understanding of the many facets of STEM research and professions they can pursue, and mentors they can continue to call upon as they explore the path forward.


Day of the Young Combatant and permanent insurrection.
March 29: Commemorating in the streets.
A date that does not go unnoticed for society as a whole, for better or for worse, is commented on and should be felt because it is inevitably a day that breaks with the everyday normality and that is seen in the streets, in high schools and universities, in workplaces, in the city centers and also in the barrios and towns.
For us anarchists, March 29 is a date where memory, resistance and subversion are combined in the streets, a date on which we remember our dead comrades who died at the hands of State power…our hearts beat with the brothers Vergara Toledo, with the guerrilla Norma Vergara and with the anarchists Jonny Cariqueo and Javier Recabarren, just to name some of the comrades who in different circumstances and years left this world some time in March and who are now impulses of destruction for old and new generations of fighters.
This March 29 we were there, taking action, fueling the fire of the barricades in the streets of Pudahuel with a diverse group of people and comrades who want this day to not go unnoticed by anyone. For what they contribute in different ways so that this occurs with the fixed idea that nobody who dies is forgotten and that the police are one of the many targets we have to attack. Because there is still much to be brought to account for those hired bastards who have taken away valuable comrades of struggle, and even more, there is much to be done against those who manipulate, control and own the territory where we live, the all powerful – our most difficult enemies.


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"Toboganul" (titlu original: "The Chute") este al 3-lea episod din al treilea sezon al serialului TV american științifico-fantastic Star Trek: Voyager și al 45-lea în total. A avut premiera la 18 septembrie 1996 pe canalul UPN.

Prezentare
Tom Paris și Harry Kim sunt captivi într-o închisoare. Tom este înjughiat atunci când încearcă să-l apere pe Kim, lăsându-l pe acesta să găsească singur un plan de evadare. În același timp, Voyager încearcă să găsească o cale de a le dovedi nevinovăția.

Rezumat

Actori ocazionali
 Don McManus - Zio
 Robert Pine - Ambassador Liria
 James Parks - Vel
 Ed Trotta - Pit
 Beans Morocco - Rib
 Rosemary Morgan - Piri

Note

Legături externe

Episoade din Star Trek: Voyager
Episoade de televiziune din 1996

redpajama_set_name: RedPajamaWikipedia


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Weekend Box Office Report: The Box Office Goes 'Home'
In one of the strongest box office weekends of 2015 so far, both Home and Get Hard opened strong while Insurgent and Cinderella continued to perform well. This was the rare weekend that literally offered something for everyone, with R-rated comedies and animated family fare exceeding expectations.
Film Weekend Per Screen
1 Home $54,000,000 $14,563 $54,000,000
2 Get Hard $34,610,000 $10,901 $34,610,000
3 Insurgent $22,075,000 (-57.8) $5,697 $86,394,000
4 Cinderella $17,515,000 (-49.9) $4,591 $150,022,000
5 It Follows $4,021,000 (+1,065.9)
$3,301 $4,755,000
6 Kingsman: The Secret Service $3,050,000 (-34.1) $1,709 $119,424,000
7 Run All Night $2,205,000 (-56.2) $928 $23,823,000
8 The Second Best Exotic Marigold Hotel $2,185,000 (-42.5) $1,459 $28,135,000
9 Do You Believe? $2,150,000 (-40.1) $1,586 $7,052,000
10 The Gunman $2,045,000 (-59.3) $726 $8,810,000
Home opened in first place with $54 million, an impressive number for any movie but especially impressive when you realize that it opened to more money than last year's How to Train Your Dragon 2. Yes, this is the exceedingly rare case of an original film making more money than a sequel (and it will hopefully teach DreamWorks a valuable lesson). Home shouldn't have a problem hitting $150 million by default, but if families really respond to it, it should have a shot at $200 million.
In second place, the combined star power of Will Ferrell and Kevin Hart propelled Get Hard to a $34 million opening. That's the biggest opening weekend for Ferrell in five years and a pretty standard opening for Hart, who is no stranger to big box office these days. That R-rating may slow the film down in the weeks ahead, but it should fall between $80 and $100 million by default.
In third place, Insurgent took the expected tumble for any film with a large opening, grossing $22 million for a current total of $86 million. It still has a few weeks to go before it reaches Divergent's $150 million gross, but it should be able to match it at the very least. It's not going to do Hunger Games business, but there's nothing wrong with a modest success, especially when the original budget doesn't break the bank.
Meanwhile, Cinderella passed the $150 million mark in its third weekend, grossing $17 million. At this rate, it should hit $200 million before the end of April, but it probably won't go much farther than that. And that's okay! $200 million for a "girl" movie is just further proof that both chromosomes go to the theaters and that studios should stop catering to teenage boys all the time.
And that brings us to fifth place and the biggest question mark of the weekend. The horror movie It Follows expanded from limited release and made $4 million, a totally respectable number for a tiny indie from a niche distributor but a disastrous number for a much-hyped horror movie that has received quite the marketing push in the past weeks. If the original VOD release had gone as planned, would It Follows have done better? Or would the numbers have been roughly the same? We don't know. Whether or not this gross is a little disappointing or totally disastrous is a matter of perspective.
The usual suspects rounded out the rest of the top 10, with Kingsman: The Secret Service leading the pack. Right below it, Run All Night continued to bomb, The Second Best Exotic Marigold Hotel continued its slow but steady march to being a small hit, and The Gunman stumbled, gasping its last breath before it vanishes from theaters in the coming days.
Source: Weekend Box Office Report: The Box Office Goes 'Home'
Categories: Duluth / Superior News


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Men's and Women's Basketball Preview
Parker Burman – Staff Writer
Both the Gustavus men's and women's basketball teams opened up their seasons this past week. The men hosted UW-River Falls, while the women went on the road to start the year against UW-Stout. At home the men fought a back and forth battle, which ended in a 62-58 defeat to start the year, while the women started off strong with a 72-53 victory.
"It feels great! There is a lot of excitement expressed in our program not only by the coaches but by the players as well. Every basketball player knows that there is no feeling that can match an opening night," Sophomore Spencer Swanson said.
In the men's game it was a struggle for both sides to find offensive traction as it took over two minutes for the first points to be scored in the game. Swanson put the Gusties on his back as he single-handedly scored Gustavus' first eight points. Gustavus built up a 15-7 lead at the 12:22 mark, but this lead evaporated quickly after as River Falls went on a 10 point unanswered scoring streak.
"We were honestly just really excited to just be back playing in front of our friends and family. Obviously the goal was to win but also just to show ourselves that we are capable of competing against a really good team," Senior Jordan Schommer said.
Gustavus was outscored 28-8 in the last 12 minutes of the half, leading to a 35-23 halftime deficit. This River Falls lead only grew in the second half as they led by 16 points with a score of 47-31 with 12:19 left in the game. This lead would be insurmountable for the Gustavus offense- though they only fell by four points.
"We came up a bit short but it was still a great opportunity for us to learn and grow. [I'm] proud of how we came out in the second half and did not back down and continued to fight till the end. It really showed the grit and fight this team has," Schommer said.
The Gustavus women fared better than the men as they were able to show off their dominance in their 72-53 victory. Their win started early, as the Gustie offense put up 20 points in the first quarter while the defense allowed Stout just four points.
"Defensively we came out strong. Only allowing 4 points in the first quarter set the tone right away. Defense is something we really focus on and take pride in as a team, so we look to hold a team to a minimum of points and build off of that. Also, we shot the ball super well which is always a plus. If you lockdown on defense and shoot well, it's amazing what a team can do," Junior Izzy Quick said.
Going into halftime, the Gusties almost matched their first half offensive production, putting up an additional 19 points. The defense was not able to match their high level of dominance in the second quarter but still only allowed 16 points to lead 39-20.
The second half was much of the same, though Stout was able to cut the Gustie lead down to 18 points. However, this was as small as the deficit would get. Gustavus closed out quarter three with a 26 point lead. All of this led the Gusties to their 72-53 victory to open the year.
Senior Anna Sanders led the team in scoring with 16 points while teammate Sophomore Kylie Baranick was hot on her tail with 15 of her own. Quick finished third in points on the team with 10, dealing out an assist and picking up three rebounds.
"Starting the season off with a win was super encouraging for us, but also a good learning opportunity. We got to see how much we have improved since our first season playing together, and since our team is almost the same as last year, it's super exciting to see how we can use this as a starting point and continue to build off of it," Quick said.
WIth a full season ahead of them, both the Gustavus men and women will be looking to make deep runs in the MIAC and hopefully into the NCAA Tournament.
"I think everyone's main goal for their sports season is to bring a MIAC Championship to Gustavus and as much as that is in our vision, we have plenty of other goals for the year. As a team, we want to show lots of progress on and off the court. I think we separate from a lot of other schools because we focus on development as athletes and humans. Regardless of what our record says, our goal is to always be a family of Gusties," Swanson said.
"The main goals for this season is to go back to the tournament, but also to win the conference. Last year we won the playoffs, which was great, but we didn't win the conference. Also, if fortunate enough to make it back to the tournament, we want to make it past the first round. The road to Dallas is something we always talk about, and I think this team is very special and has the talent, chemistry, and trust in one another to do so," Quick said.
David Eide November 30, 2022
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