more typo

hiromacros.sty

@@ -93,7 +93,7 @@
 \def\hilb{\ensuremath{\mathcal{H}}}
 
 % fixme
-\newcommand{\fixme}[1]{\marginpar{\tiny\textcolor{red}{#1}}}
+\newcommand{\fixme}[1]{} %{\marginpar{\tiny\textcolor{red}{#1}}}
 
 % HOPS/NMQSD
 \def\sys{\ensuremath{\mathrm{S}}}
@@ -140,3 +140,28 @@
 \newcommand{\plot}[1]{%
   \includegraphics[draft=false]{./figs/#1.pdf}}
 \newcommand{\tval}[1]{{\input{./values/#1.tex}}}
+
+%% citing "in ref"
+\NewBibliographyString{refname}
+\NewBibliographyString{refsname}
+\DefineBibliographyStrings{english}{%
+  refname = {Ref\adddot},
+  refsname = {Refs\adddot}
+}
+
+\DeclareCiteCommand{\refcite}
+  {%
+  \ifnum\thecitetotal=1
+    \bibstring{refname}%
+  \else%
+    \bibstring{refsname}%
+  \fi%
+  \addspace\bibopenbracket%
+  \usebibmacro{cite:init}%
+   \usebibmacro{prenote}}
+  {\usebibmacro{citeindex}%
+   \usebibmacro{cite:comp}}
+  {}
+  {\usebibmacro{cite:dump}%
+   \usebibmacro{postnote}%
+   \bibclosebracket}

hirostyle.sty

@@ -82,30 +82,4 @@ linkcolor=blue,
 % cursive bold in maths
 \unimathsetup{math-style=TeX,bold-style=ISO}
 
-%% citing "in ref"
-\NewBibliographyString{refname}
-\NewBibliographyString{refsname}
-\DefineBibliographyStrings{english}{%
-  refname = {Ref\adddot},
-  refsname = {Refs\adddot}
-}
-
-\DeclareCiteCommand{\refcite}
-  {%
-  \ifnum\thecitetotal=1
-    \bibstring{refname}%
-  \else%
-    \bibstring{refsname}%
-  \fi%
-  \addspace\bibopenbracket%
-  \usebibmacro{cite:init}%
-   \usebibmacro{prenote}}
-  {\usebibmacro{citeindex}%
-   \usebibmacro{cite:comp}}
-  {}
-  {\usebibmacro{cite:dump}%
-   \usebibmacro{postnote}%
-   \bibclosebracket}
-
-
 \recalctypearea

poster/poster_abstract.tex

@@ -38,7 +38,7 @@ non-Markovian strongly coupled open systems. Without modification of
 the core method, it is possible to calculate the interaction energy
 and the bath energy change. This is due to HOPS' foundation on the
 global dynamics of the system and the bath in contrast to
-master-equation methods. We extended the result in~\cite{Kato2016Dec}
+master-equation methods. We extended the result in \refcite{Kato2016Dec}
 for the Hierarchical Equations Of Motion method to arbitrary
 modulations of system and coupling inheriting all the advantages of
 the HOPS method.

src/flow.tex

@@ -136,7 +136,7 @@ Defining
   \label{eq:defdop}
 D_t = ∫_0^t\dd{s} \alpha(t-s)\fdv{η^\ast_s}
 \end{equation}
-as in~\cite{Suess2014Oct} we find
+as in \refcite{Suess2014Oct} we find
 \begin{equation}
   \label{eq:final_flow_nmqsd}
   J(t) = -\i \mathcal{M}_{η^\ast}\bra{\psi(η,
@@ -511,7 +511,7 @@ general.  We refer to \cref{sec:hops_multibath} for an review of the
 NMQSD theory and HOPS method for multiple baths.
 
 Because the bath energy change is being calculated directly and not
-through energy conservation as in~\cite{Kato2016Dec}, we find
+through energy conservation as in \refcite{Kato2016Dec}, we find
 \begin{equation}
   \label{eq:general_n_flow}
   J_n=-\dv{\ev{H_\bath^{(n)}}}{t} = \iu\ev{[H_\bath^{(n)},

src/intro.tex

@@ -319,7 +319,7 @@ arrive at an equation for \(\ket{ψ(t,\vb{z}^{\ast})}\)
 From this point on there are multiple avenues open to us. We choose
 the canonical one of \cite{Strunz2001Habil}, but there is also a
 time-discrete derivation, that avoids functional derivatives,
-in~\cite{Hartmann2021Aug}.
+in \refcite{Hartmann2021Aug}.
 
 We shift the perspective and define~\cite{RichardDiss,Strunz2001Habil}
 \begin{equation}
@@ -486,7 +486,7 @@ We call \cref{eq:singlehops} the \emph{Hierarchy of Pure States}
 because each hierarchy state couples only to the hierarchy states one
 level above and one level below. This is similar to the
 \emph{Hierarchical Equations of Motion} (HEOM) approach used
-in~\cite{Kato2016Dec}, but with the advantage of reducing the
+in \refcite{Kato2016Dec}, but with the advantage of reducing the
 dimensionality from \(\dim{\hilb_{\sys}}^{2}\) to
 \(\dim{\hilb_{\sys}}\) by treating pure states instead of density
 matrices.

src/num_results.tex

@@ -109,7 +109,7 @@ the ``Markovianity'' of the bath.
 
 The ohmic spectral density models an environment with a physical
 energy spectrum that is bounded from below and allows the application
-of the finite temperature method described in~\cite{RichardDiss} and
+of the finite temperature method described in \refcite{RichardDiss} and
 \cref{sec:lin_finite}. Also, \(J(0) = 0\) ensures that there is a
 unique zero temperature state of the bath. In~\cite{Kolar2012Aug} it
 is argued (under weak coupling assumptions), that \(J(ω)\approx ω^γ\)
@@ -122,7 +122,7 @@ It may be remarked, that~\cref{eq:ohmic_bcf} does not correspond to a
 simple sum of exponentials. As such it exercises the HOPS method and
 serves as a model for a general bath correlation function. For use
 with HOPS, a sum of exponentials must be fitted to the BCF. This has
-been done in~\cite{RichardDiss,Hartmann2021Aug}. In
+been done in \refcite{RichardDiss,Hartmann2021Aug}. In
 \cref{sec:hopsvsanalyt} we will see, that this is indeed a valid
 strategy for the application of \cref{chap:flow}.
 
@@ -753,7 +753,7 @@ the stochastic process we chose the cutoff \(\abs{\vb{k}} \leq 4\)
 (simplex truncation\footnote{see \cref{sec:hops_basics}}),
 \(N=4.5 \cdot 10^5\) trajectories and an Ohmic BCF with \(α(0)=1.6\)
 and \(ω_c=4\).  The sampling method uses the ``Fast Fourier
-Transform'' (FFT) as described in~\cite{RichardDiss}. As the system
+Transform'' (FFT) as described in \refcite{RichardDiss}. As the system
 Hilbert space dimension is small, a BCF expansion with seven terms was
 employed~\cite{Hartmann2021Aug,RichardDiss}.
 
@@ -855,7 +855,7 @@ convergence as is also demonstrated in
 \subsection{Hierarchy Truncation}
 \label{sec:trunc}
 As the systematics of the truncation depth have already been studied
-thoroughly in~\cite{RichardDiss,Hartmann2021Aug}, we will keep the
+thoroughly in \refcite{RichardDiss,Hartmann2021Aug}, we will keep the
 discussion short.  We chose \(N=4.5 \cdot 10^5\) trajectories and an
 Ohmic BCF with \(α(0)=0.8\) and \(ω_c=2\). Again, a BCF expansion with
 seven terms has been used. The coupling strength has been chosen with

src/thermo.tex

@@ -73,7 +73,7 @@ change over one cycle.
 
 In \cref{sec:operational_thermo} a Gibbs like inequality for an
 arbitrary number of baths is derived as a slight generalization of the
-derivation in~\cite{Kato2016Dec}. The left hand side of this
+derivation in \refcite{Kato2016Dec}. The left hand side of this
 inequality can be associated with a thermodynamic cost that should be
 minimized for optimal efficiency.
 
@@ -112,7 +112,7 @@ where \(n<∞\) is the Hilbert space dimension. This condition is both
 necessary and sufficient. Examples of passive states are the state of
 the micro-canonical ensemble or Gibbs states. Gibbs states are further
 distinguished by additional features described
-in~\cite{Lenard1978Dec}, which can be connected to formulations of the
+in \refcite{Lenard1978Dec}, which can be connected to formulations of the
 zeroth and second laws of thermodynamics.
 
 One of these properties is complete passivity. Completely passive
@@ -289,7 +289,7 @@ bath properties except the temperature. It is therefore reasonable to
 expected that it is also valid for an infinite bath.
 
 Interestingly, a saturation of \cref{eq:thermo_ergo_bound} is achieved
-in~\cite{Skrzypczyk2014Jun} with a continuous qubit
+in \refcite{Skrzypczyk2014Jun} with a continuous qubit
 bath. In~\cite{Lobejko2021Feb} a more generic argument is made in a
 similar setting. Both propose concrete protocols within the bounds of
 thermal operations and by considering explicit work reservoirs. In
@@ -672,7 +672,7 @@ energy that can be extracted out of the system in relation to the
 energy that is simply transferred between the baths.
 
 An argument based on entropy may be made for the periodic steady state
-as was shown in~\cite{Kato2016Dec} and is reproduced here with the
+as was shown in \refcite{Kato2016Dec} and is reproduced here with the
 slight generalization of multiple baths and modulated coupling. We
 will find a Clausius like form of the second law. The left hand side
 of this inequality can then be interpreted as thermodynamic cost of
@@ -789,7 +789,7 @@ If one defines heat in this
 way~\cite{Kato2016Dec,Riechers2021Apr,Strasberg2021Aug},
 \cref{eq:secondlaw_cyclic} amounts to the Clausius inequality. The
 definition of heat as bath energy change is corroborated
-in~\cite{Esposito2015Dec} where it is shown, ableit for fermionic
+in \refcite{Esposito2015Dec} where it is shown, ableit for fermionic
 baths, that a definition of heat involving any nonzero fraction of the
 interaction energy will lead to the internal energy (as defined by the
 first law) not being an exact differential.
@@ -1391,7 +1391,7 @@ however, we find that also the modulation of the interaction, i.e. the
 coupling and decoupling, figures into the total power and reduces the
 energy output. In a weak coupling scheme, this contribution can be
 neglected. Not so however in the generic case presented here. A
-similar result was found in~\cite{Wiedmann2021Jun}.
+similar result was found in \refcite{Wiedmann2021Jun}.
 
 The mean power output of this cycle is
 \(\bar{P}=0.002468\pm 0.000021\) with an efficiency, as defined in

talk/index.tex

@@ -817,7 +817,7 @@ labelformat=brace, position=top]{subcaption}
   \(J(ω) = π ∑_λ\abs{g_λ}^2δ(ω-ω_λ)\)).
 \end{frame}
 \begin{frame}{Fock-Space Embedding}
-  As in~\cite{Gao2021Sep} we can define
+  As in \refcite{Gao2021Sep} we can define
   \begin{equation}
     \label{eq:fockpsi}
     \ket{Ψ} = \sum_\kmat\ket{\psi^\kmat}\otimes \ket{\kmat}