Subsystem Trace Distance in Quantum Field Theory

TL;DR

This paper introduces a systematic method to compute the trace distance between reduced density matrices in 1+1 dimensional quantum field theories, with applications to conformal field theories and spin chain models.

Contribution

It develops a novel approach using path integrals and replica tricks to calculate trace distances, providing universal formulas and numerical validation.

Findings

Derived universal leading order trace distance for short intervals in CFTs.

Calculated trace distances for low-lying states in free boson and fermion theories.

Confirmed analytic results with numerical simulations in spin chain models.

Abstract

We develop a systematic method to calculate the trace distance between two reduced density matrices in 1+1 dimensional quantum field theories. The approach exploits the path integral representation of the reduced density matrices and an ad hoc replica trick. We then extensively apply this method to the calculation of the distance between reduced density matrices of one interval of length $\ell$ in eigenstates of conformal field theories. When the interval is short, using the operator product expansion of twist operators, we obtain a universal form for the leading order in $\ell$ of the trace distance. We compute the trace distances among the reduced density matrices of several low lying states in two-dimensional free massless boson and fermion theories. We compare our analytic conformal results with numerical calculations in XX and Ising spin chains finding perfect agreement.

Figures

Equations

$$D_n(\rho ,\sigma )=\frac{1}{2^{1/n}}\Vert \rho -\sigma {\Vert }_n,$$

$$\mathrm{tr}{\rho }_A^n=⟨\mathcal{T}(\ell ,\ell )\tilde{\mathcal{T}}(0,0){⟩}_{{\rho }_n}.$$

$$D_1({\rho }_A,{\sigma }_A)=\frac{1}{2}\underset{n_e\to 1}{\lim }\mathrm{tr}({\rho }_A-{\sigma }_A{)}^{n_e}.$$

$$\mathrm{tr}({\rho }_A-{\sigma }_A{)}^n=\sum _{\mathcal{S}}(-{)}^{|\mathcal{S}|}\mathrm{tr}\left({\rho }_{0_{\mathcal{S}}}\cdots {\rho }_{(n-1{)}_{\mathcal{S}}}\right),$$

$$\mathrm{tr}\left({\rho }_{0_{\mathcal{S}}}\cdots {\rho }_{{(n-1)}_{\mathcal{S}}}\right)=⟨\mathcal{T}(\ell ,\ell )\tilde{\mathcal{T}}(0,0){⟩}_{{\otimes }_j{\rho }_{j_{\mathcal{S}}}}.$$

$$f(z)={\left(\frac{z-e^{2\pi \mathrm{i}\ell /L}}{z-1}\right)}^{1/n}.$$

$$\mathrm{tr}(\rho_{\mathcal{X}}-\rho_{\mathcal{Y}})^{n}=c_{n}\Big{(}\frac{L}{\pi\epsilon}\sin\frac{\pi\ell}{L}\Big{)}^{-4h_{n}}\\ \sum_{\mathcal{S}}\Big{\{}(-)^{|\mathcal{S}|}\mathrm{i}^{2(|\bar{\mathcal{S}}|s_{\mathcal{X}}+|\mathcal{S}|s_{\mathcal{Y}})}\Big{(}\frac{2}{n}\sin\frac{\pi\ell}{L}\Big{)}^{2(|\bar{\mathcal{S}}|\Delta_{\mathcal{X}}+|\mathcal{S}|\Delta_{\mathcal{Y}})}\\ \times\Big{\langle}\Big{[}\prod_{j\in\bar{\mathcal{S}}}\Big{(}f_{j,\ell}^{h_{\mathcal{X}}}\bar{f}_{j,\ell}^{\bar{h}_{\mathcal{X}}}f_{j}^{h_{\mathcal{X}}}\bar{f}_{j}^{\bar{h}_{\mathcal{X}}}\mathcal{X}(f_{j,\ell},\bar{f}_{j,\ell})\mathcal{X}^{\dagger}(f_{j},\bar{f}_{j})\Big{)}\Big{]}\\ \times\Big{[}\prod_{j\in\mathcal{S}}\Big{(}f_{j,\ell}^{h_{\mathcal{Y}}}\bar{f}_{j,\ell}^{\bar{h}_{\mathcal{Y}}}f_{j}^{h_{\mathcal{Y}}}\bar{f}_{j}^{\bar{h}_{\mathcal{Y}}}\mathcal{Y}(f_{j,\ell},\bar{f}_{j,\ell})\mathcal{Y}^{\dagger}(f_{j},\bar{f}_{j})\Big{)}\Big{]}\Big{\rangle}_{\mathbb{C}}\Big{\}}.$$

$${\mathcal{D}}_n(\rho ,\sigma )=\frac{\mathrm{tr}{\left(\rho -\sigma \right)}^n}{\mathrm{tr}{\rho }^n},$$

$$D_1(\rho ,\sigma )=\frac{1}{2}\underset{n_e\to 1}{\lim }{\mathcal{D}}_{n_e}(\rho ,\sigma ).$$

$$\mathrm{tr}\rho_{A}^{n}=c_{n}\Big{(}\frac{\ell}{\epsilon}\Big{)}^{-4h_{n}}\Big{[}1+\sum_{k=1}^{n}\sum_{\{\mathcal{X}_{1},\cdots,\mathcal{X}_{k}\}}\ell^{\Delta_{\mathcal{X}_{1}}+\cdots+\Delta_{\mathcal{X}_{n}}}\\ \times b_{\mathcal{X}_{1}\cdots\mathcal{X}_{k}}\langle\mathcal{X}_{1}\rangle_{\rho}\cdots\langle\mathcal{X}_{k}\rangle_{\rho}\Big{]}.$$

$$\displaystyle\mathrm{tr}(\rho_{A}-\sigma_{A})^{n}=c_{n}\Big{(}\frac{\ell}{\epsilon}\Big{)}^{-4h_{n}}\sum_{\{\mathcal{X}_{1},\cdots,\mathcal{X}_{n}\}}\big{[}\ell^{\Delta_{\mathcal{X}_{1}}+\cdots+\Delta_{\mathcal{X}_{k}}}$$

$$\displaystyle~{}\times b_{\mathcal{X}_{1}\cdots\mathcal{X}_{n}}\big{(}\langle\mathcal{X}_{1}\rangle_{\rho}-\langle\mathcal{X}_{1}\rangle_{\sigma}\big{)}\cdots\big{(}\langle\mathcal{X}_{n}\rangle_{\rho}-\langle\mathcal{X}_{n}\rangle_{\sigma}\big{)}\big{]}.$$

$$⟨\varphi {⟩}_{\rho }-⟨\varphi {⟩}_{\sigma }\ne 0,$$

$$\frac{\mathrm{tr}(\rho_{A}-\sigma_{A})^{n_{e}}}{\mathrm{tr}\rho_{A}^{n_{e}}}=\ell^{n_{e}\Delta_{\phi}}b_{\phi\cdots\phi}\big{(}\langle\phi\rangle_{\rho}-\langle\phi\rangle_{\sigma}\big{)}^{n_{e}}+o(\ell^{n_{e}\Delta_{\phi}}),$$

$$D_1({\rho }_A,{\sigma }_A)=\frac{x_{\varphi }|⟨\varphi {⟩}_{\rho }-⟨\varphi {⟩}_{\sigma }|}{2}{\ell }^{{\Delta }_{\varphi }}+o({\ell }^{{\Delta }_{\varphi }}),$$

$$x_{\phi}=\lim_{p\to 1/2}\frac{\mathrm{i}^{2ps_{\phi}}}{(2p)^{2p\Delta_{\phi}}}\Big{\langle}\prod_{j=0}^{2p-1}\big{[}\mathrm{e}^{\frac{\pi\mathrm{i}j}{p}s_{\phi}}\phi(\mathrm{e}^{\frac{\pi\mathrm{i}j}{p}},\mathrm{e}^{-\frac{\pi\mathrm{i}j}{p}})\big{]}\Big{\rangle}_{\mathbb{C}}.$$

$$x_{\varphi }\le x_{\max }({\Delta }_{\varphi })=\sqrt{\frac{{\pi }^{1/2}\Gamma ({\Delta }_{\varphi }+1)}{2^{2{\Delta }_{\varphi }+1}\Gamma ({\Delta }_{\varphi }+\frac{3}{2})}},$$

$$\begin{gathered} {\mathcal{D}}_n[\Delta \alpha ]\equiv {\mathcal{D}}_n({\rho }_{\alpha ,\bar{\alpha }},{\rho }_{{\alpha }^{\prime },{\bar{\alpha }}^{\prime }})= \\ \sum _{k=0}^n(-{)}^k\sum _{0\le j_1<\cdots <j_k\le n-1}{d}_n(\{j_1,\cdots ,j_k\}{)}^{\Delta \alpha }, \end{gathered}$$

$$d_{n}(\mathcal{S})=\Big{(}\frac{\sin{\frac{\pi\ell}{L}}}{n\sin{\frac{\pi\ell}{nL}}}\Big{)}^{|\mathcal{S}|}\times\\ \times\prod^{j_{1}<j_{2}}_{j_{1},j_{2}\in\mathcal{S}}\frac{\sin^{2}\frac{\pi(j_{1}-j_{2})}{n}}{\sin\frac{\pi(j_{1}-j_{2}+\ell/L)}{n}\sin\frac{\pi(j_{1}-j_{2}-\ell/L)}{n}},$$

$$\log\mathcal{D}_{n}[1]=n\log(2\pi)-2\!\int_{0}^{\infty}\!\!\frac{dt}{t}\Big{\{}\frac{1}{\mathrm{e}^{t}-1}\\ \times\Big{[}\frac{(\mathrm{e}^{\frac{t\ell}{2L}}-1)\big{(}1+\mathrm{e}^{t}\mathrm{e}^{-\frac{t\ell}{2L}}\big{)}}{2\sinh\big{(}\frac{t\ell}{2nL}\big{)}}-n\Big{]}-\frac{n}{2}\Big{\}},$$

$$\underset{n_e\to 1}{\lim }{\mathcal{D}}_{n_e}[1]=2\ell /L.$$

$$\displaystyle D_{1}(\rho_{{\alpha,\bar{\alpha}}},\rho_{{\alpha^{\prime},\bar{\alpha}}})=\frac{|\alpha-\alpha^{\prime}|\ell}{L}+o\Big{(}\frac{\ell}{L}\Big{)},$$

$$\displaystyle D_{1}(\rho_{{\alpha,\bar{\alpha}}},\rho_{{\alpha,\bar{\alpha}^{\prime}}})=\frac{|\bar{\alpha}-\bar{\alpha}^{\prime}|\ell}{L}+o\Big{(}\frac{\ell}{L}\Big{)}.$$

$$\displaystyle D_{1}(\rho_{J},\rho_{{\alpha,0}})=D_{1}(\rho_{\bar{J}},\rho_{{0,\alpha}})=\frac{|\alpha|\ell}{L}+o\Big{(}\frac{\ell}{L}\Big{)},$$

$$\displaystyle D_{1}(\rho_{J},\rho_{{0,\bar{\alpha}}})=D_{1}(\rho_{\bar{J}},\rho_{{\bar{\alpha},0}})=\frac{|\bar{\alpha}|\ell}{L}+o\Big{(}\frac{\ell}{L}\Big{)}.$$

Full text

During recent times, in several disconnected fields of physics emerged the necessity to characterise the properties of extended subsystems rather than of the entire system. A first important example is the non-equilibrium dynamics of isolated quantum systems: while the whole system remains in a pure state, subsystems are described by statistical ensembles for large times bs-08 ; gogolin-2015 ; calabrese-2016 ; vidmar-2016 ; ef-16 ; dls-13 ; kaufman-2016 ; ac-17 . Another subject where the physics of the subsystem matters is the black hole information loss paradox h-74 and its relation to the distinguishability of states in gauge field theories through the gauge/gravity duality Maldacena:1997re ; rt-06 ; r-10 ; m1 ; ms-13 ; Fitzpatrick:2016ive . Indeed, the large interest in the physics of subsystems was the main reason of the vast theoretical intro1 ; intro2 ; intro3 and experimental exp1 ; kaufman-2016 ; evdcz-18 ; lukin-18 activity aimed to characterise the entanglement of extended quantum systems. Yet, it is very important not only to have information about the subsystems, but also to have a notion of distance between the subsystems’ configurations, more precisely between the reduced density matrices (RDM) of a subsystem in two different states.

Several different measures of the distance between density matrices exist and are widely used in quantum information nc-book ; watrous-book . For example, given two density matrices $\rho$ and $\sigma$ acting on the same Hilbert space, a family of distances, depending on a continuous parameter $n$, is provided by the $n$-distances

[TABLE]

where the $n$-norm is $\|\Lambda\|_{n}=(\sum_{i}\lambda_{i}^{n})^{1/n}$ with $\lambda_{i}$ being the singular values of $\Lambda$, i.e., the eigenvalues of $\sqrt{\Lambda^{\dagger}\Lambda}$. When $\Lambda$ is Hermitian, $\lambda_{i}$ are just the absolute values of the eigenvalues of $\Lambda$. (The normalization $2^{1/n}$ ensures $0\leq D_{n}(\rho,\sigma)\leq 1$.) In finite dimensional Hilbert spaces all norms are equivalent (in the sense that they bound each other), but this ceases to be the case for infinite dimensional spaces and we are interested in quantum field theories (QFT). Furthermore, even in finite dimensions, the bounds between norms depend on the dimension and so the distances are not on equal footing when comparing subsystems of different sizes. There are several reasons why the trace distance $D_{1}$ is special, e.g. the difference of expectation values of an operator $O$ in different states is bounded as $|\mathrm{tr}(\rho-\sigma)O|\leq D_{1}(\rho,\sigma)||O||_{1}$, and the bound has no factor depending on the Hilbert space dimension, as it would be the case for other norms, see e.g. fe-13b .

It is however extremely difficult to evaluate analytically $D_{1}$: even for Gaussian states there is no way to compute it from the two-point correlators (see e.g. fe-13b ). This is indeed one of the reasons why for quantum field theories there has been a huge activity hol-rel-entropy ; lashkari2014 ; bhm-14 ; lashkari2016 ; rc-17 ; su-16 ; su-17 ; casini-2016 ; Nakagawa:2017fzo ; mrc-18 in quantifying the relative entropy $S(\rho\|\sigma)=\mathrm{tr}(\rho\log\rho)-\mathrm{tr}(\rho\log\sigma)$, which provides an idea about the distance of $\rho$ and $\sigma$, but it is not even a metric since it is not symmetrical.

In this Letter we develop a systematic method to calculate the trace distance between two RDMs in quantum field theories. This is based on an ad hoc replica trick: we first calculate the $n$-distance (1) for a general even integer $n$, we analytically continue it to real $n$, and finally we take the limit $n\to 1$ to get the trace distance. (This trick is reminiscent of the one for entanglement negativity in QFT cct-12 .) For even $n$, we express $D_{n}$ as a correlation function in a replicated worldsheet, that, in 1+1 dimensions, can be written in terms of the twist operators of Refs. cc-04 ; cc-09 ; ccd-08 . We will then exploit this method to provide very general results for the distance between primary states in 2D conformal field theories (CFT) and use the operator product expansion (OPE) of the twist fields headrick ; cct-11 ; gr-12 ; cz-13 ; cwz-16 ; lwz-16 ; hlz-17 for short intervals. In this Letter we just introduce our replica approach and show how it works with a few examples. Most details are left to a technical forthcoming publication work-td .

General description in QFT.

We consider a generic QFT in a state described by the density matrix $\rho$ and we focus on a spatial subsystem $A$. The reduced density matrix $\rho_{A}=\mathrm{tr}_{\bar{A}}\rho$ is obtained by tracing out the degrees of freedom of $\bar{A}$, the complement of $A$. The bipartite entanglement between $A$ and $\bar{A}$ may be measured by the celebrated entanglement entropy $S_{A}=-\mathrm{tr}(\rho_{A}\log\rho_{A})$ which can be obtained from the replica limit of $\mathrm{tr}\rho_{A}^{n}$ cc-09 ; cc-04 . In the path integral Euclidean formalism and for $n\in\mathbb{N}$, such traces correspond to partition functions on an $n$-sheeted Riemann surface (see Fig. 1, left), with the sheet $j$ representing $\rho_{A,j}$ (the $j$-th copy of the state $\rho_{A}$ of the initial QFT). Moreover, for one interval embedded in a 1D systems (equivalently 2D QFT), the same quantities can be interpreted as two-point functions (or, more generally, $2m$-point functions if the subsystem consists of $m$ disjoint intervals) evaluated in the state $\rho_{n}=\otimes_{j=0}^{n-1}\rho_{A,j}$ of the corresponding $n$-fold theory cc-04 ; ccd-08

[TABLE]

${\mathcal{T}}$ and $\tilde{\mathcal{T}}$ are called twist and antitwist operators respectively. This form is particularly useful in the context of CFT, where ${\mathcal{T}}$ and $\tilde{\mathcal{T}}$ are primary operators of the $n$-fold theory (dubbed CFTn) with conformal weights $h_{n}=\bar{h}_{n}=\frac{c(n^{2}-1)}{24n}$ cc-04 . Here $c$ is the central charge of the single-copy CFT. For an interval of length $\ell$ in an infinite system, this leads to the famous result $\mathrm{tr}\rho_{A}^{n}=c_{n}({\ell}/{\epsilon})^{-4h_{n}}$ where $c_{n}$ is the normalization constant cc-09 ($c_{1}=1$) of the twist operators and $\epsilon$ the UV cutoff.

Here, we are interested in the trace distance (i.e. (1) for $n=1$) between two generic RDMs $\rho_{A},\sigma_{A}$. For an arbitrary even integer $n_{e}$ we have $\|\rho_{A}-\sigma_{A}\|_{n_{e}}^{n_{e}}=\mathrm{tr}(\rho_{A}-\sigma_{A})^{n_{e}}$. Therefore, if we are able to compute $\mathrm{tr}(\rho_{A}-\sigma_{A})^{n_{e}}$ and analytically continue it as a function of $n_{e}$ from even integers to generic real values, then the trace distance is obtained via the following replica trick

[TABLE]

We stress that for odd $n_{o}$ instead, $\mathrm{tr}(\rho_{A}-\sigma_{A})^{n_{o}}$ does not provide the $n_{o}$-distance. Hence the limit $n_{o}\to 1$ just gives the trivial result $\mathrm{tr}(\rho_{A}-\sigma_{A})=0$, in full analogy to the negativity replica trick cct-12 .

To proceed, we note that $\mathrm{tr}(\rho_{A}-\sigma_{A})^{n}$ may be expanded as

[TABLE]

where the summation $\mathcal{S}$ is over all the subsets of $\mathcal{S}_{0}=\{0,\cdots,n-1\}$, $|\mathcal{S}|$ is the cardinality of $\mathcal{S}$ and $\rho_{j_{\mathcal{S}}}=\sigma_{A}$ if $j\in\mathcal{S}$ and $\rho_{A}$ otherwise. Crucially, each term in the sum appearing in the r.h.s. of Eq. (4) is related to a partition function on an $n$-sheeted Riemann surface (see Fig. 1, right) and, again, in a 2D QFT, it can be written as a two-point function of twist fields (cfr., e.g., dei-18 )

[TABLE]

Such objects are the same appearing in the replica trick for the relative entropy lashkari2014 ; lashkari2016 and in some cases have been explicitly computed lashkari2014 ; lashkari2016 ; su-16 ; su-17 ; rc-17 . Still, performing the sum in Eq. (4) and obtaining its analytic continuation is not an easy task.

Trace distance in 2D CFT.

We now consider a 1D system whose scaling limit is described by a 2D CFT. We focus on periodic systems of total length $L$ and on a subsystem being an interval of length $\ell$ (say $A=[0,\ell]$). In Euclidean path integral, the CFT is described by the complex coordinate $z=x+\mathrm{i}t$ (and its conjugate $\bar{z}$), with $x\in[0,L]$ and $t\in\mathbb{R}$, i.e. the worldsheet is an infinite cylinder. We consider the distance between RDMs of orthogonal eigenstates; as we shall see while the distance between the entire states is maximal, subsystems may be rather close. For a general primary operator $\mathcal{X}$ of conformal weights $(h_{\mathcal{X}},\bar{h}_{\mathcal{X}})$, scaling dimension $\Delta_{\mathcal{X}}=h_{\mathcal{X}}+\bar{h}_{\mathcal{X}}$ and spin $s_{\mathcal{X}}=h_{\mathcal{X}}-\bar{h}_{\mathcal{X}}$, we can use the state-operator correspondence to construct the ket $|\mathcal{X}\rangle$ and bra $\langle\mathcal{X}|$ states. The associated density matrix restricted to $A$ is simply $\rho_{\mathcal{X}}=\mathrm{tr}_{\bar{A}}|\mathcal{X}\rangle\langle\mathcal{X}|$. We exploit Eq. (4) to compute $\mathrm{tr}\left(\rho_{\mathcal{X}}-\rho_{\mathcal{Y}}\right)^{n}$ for two RDMs associated to two primary operators $\mathcal{X}$ and $\mathcal{Y}$. For such states, each term of the sum in the r.h.s. corresponds to a $2n$-point correlation function of the fields $\mathcal{X}$ and $\mathcal{Y}$ on the Riemann surface sierra ; berganza , which is mapped to the complex plane $\mathbb{C}$ through the map

[TABLE]

The final result for the entire sum in Eq. (4) can be written as a sum of such correlation functions and reads

[TABLE]

Here $\bar{\mathcal{S}}=\mathcal{S}_{0}/\mathcal{S}$, $f_{j}=\mathrm{e}^{\frac{2\pi\mathrm{i}j}{n}}$ and $f_{j,\ell}=\mathrm{e}^{\frac{2\pi\mathrm{i}}{n}(j+\frac{\ell}{L})}$. Note that in the limit $n\to 1$ the dependence on the ultraviolet cutoff $\epsilon$ washes out. Importantly, this means that the trace distance is cutoff independent, scale invariant (i.e., it depends on $\ell$ and $L$ only through $\ell/L$), and universal. We can also introduce scale-invariant cutoff-independent quantities for the $n$-distance as

[TABLE]

with replica limit from (3)

[TABLE]

Small interval expansion.

When the interval is short $\ell\ll L$, one can use the OPE of twist operators headrick ; cct-11 ; gr-12 ; cz-13 to expand the partition function (2) as a sum of one-point functions in CFTn. When the state $\rho$ is translational invariant, in the OPE of twist operators in (2) we only need to include the CFTn quasiprimary operators that are direct products of the nonidentity quasiprimary operators $\{{\mathcal{X}}\}$ of the original CFT, i.e. operators of the form $\mathcal{X}_{1}^{j_{1}}\cdots\mathcal{X}_{k}^{j_{k}}$ (see cwz-16 ; rtc-18 for a discussion). For example $\mathrm{tr}\rho_{A}^{n}$ is expanded as cwz-16 ; lwz-16 ; hlz-17

[TABLE]

The coefficients $b_{\mathcal{X}_{1}\cdots\mathcal{X}_{k}}$ have been defined in cwz-16 and they are related to the OPE coefficients of the CFTn operators $\mathcal{X}_{1}^{j_{1}}\cdots\mathcal{X}_{k}^{j_{k}}$.

Similarly, for the RDMs $\rho_{A}$, $\sigma_{A}$ of two translationally invariant states $\rho$, $\sigma$, following Ref. hlz-17 , one gets

[TABLE]

Given that the two states $\rho$, $\sigma$ are different, quasiprimary operators $\phi$ such that

[TABLE]

should exist. The OPE in (Small interval expansion.) is dominated by the quasiprimary operator $\phi$ satisfying (12) with the smallest scaling dimension $\Delta_{\phi}$. For simplicity, we assume that there is only a single $\phi$ with these properties (but this condition can be relaxed). The operator $\phi$ is normalized as $\langle\phi(0,0)\phi(z,\bar{z})\rangle_{\mathbb{C}}=z^{-2h_{\phi}}\bar{z}^{-2\bar{h}_{\phi}}$ and is a bosonic operator, i.e., its spin $s_{\phi}$ is an integer. Hence, for general even integer $n_{e}$, from (Small interval expansion.) we get

[TABLE]

with $\phi\cdots\phi$ denoting the direct product of $n_{e}$ $\phi$’s. In Eqs. (10), (Small interval expansion.), and (13), the $L$ dependence is hidden in $\langle\mathcal{X}_{k}\rangle_{\rho}\propto L^{-\Delta_{k}}$, making each addendum a function only of $\ell/L$.

For arbitrary $n_{e}$, (Small interval expansion.) leads to the expansion of the $n_{e}$-distance $D_{n_{e}}(\rho_{A},\sigma_{A})$ and (13) gives its leading order for a short interval. The replica limit $n_{e}\to 1$ of (13) provides a universal expression for the leading order trace distance in short interval expansion

[TABLE]

with ($n_{e}=2p$, $p\in\mathbb{N}$)

[TABLE]

This short distance result is remarkable, although it only applies to the case with no degeneracy at scaling dimension $\Delta_{\phi}$, i.e., that at scaling dimension $\Delta_{\phi}$ there only exists one quasiprimary operator $\phi$ with $\langle\phi\rangle_{\rho}-\langle\phi\rangle_{\sigma}\neq 0$. The correlation function appearing in (15) has been explicitly calculated for several operators in sierra ; berganza and analytically continued in elc-13 .

Finally, we also get an upper bound for $x_{\phi}$

[TABLE]

which depends solely on the scaling dimension. Eq. (16) follows from the Pinsker’s inequality $D(\rho,\sigma)\leq\sqrt{S(\rho\|\sigma)/2}$ and known results for the (universal) leading order of the relative entropy su-16 ; su-17 ; hlz-17 .

2D free massless boson theory.

We consider the 2D free massless boson theory compactified on circle of unit radius, corresponding to a 2D CFT with central charge $c=1$. We denote by $\varphi$, $\bar{\varphi}$ the holomorphic and anti-holomorphic parts of the scalar, respectively. The primary operators are the currents $J=\mathrm{i}\partial\varphi$, $\bar{J}=\mathrm{i}\bar{\partial}\bar{\varphi}$ with conformal weights $(1,0)$, $(0,1)$ as well as the vertex operators $V_{\alpha,\bar{\alpha}}=\exp(\mathrm{i}\alpha\varphi+\mathrm{i}\bar{\alpha}\bar{\varphi})$ with $\alpha,\bar{\alpha}=0,\pm 1,\cdots$ and conformal weights $({\alpha^{2}}/{2},{\bar{\alpha}^{2}}/{2})$. The low energy excited states are obtained by acting on the vacuum with such operators. We denote the associated RDMs as $\rho_{\alpha,\bar{\alpha}}$, $\rho_{J}$, $\rho_{\bar{J}}$ and $\rho_{0,0}=\rho_{0}$. Details about the 2D free massless boson theory can be found in DiFrancesco:1997nk ; Blumenhagen:2009zz .

We start by considering Eq. (8) for two generic vertex operators when it can be written as

[TABLE]

where $\Delta\alpha\equiv(\alpha-\alpha^{\prime})^{2}+(\bar{\alpha}-\bar{\alpha}^{\prime})^{2}$ and

[TABLE]

as a function of a given subset $\mathcal{S}$.

For $n=n_{e}$ being a fixed even integer, (17) can be easily computed and one also can derive a compact expression for it (see work-td ). Its analytic continuation from even integers to arbitrary real values, instead, is not simple. Remarkably, for $\Delta\alpha=1$, we were able to find the full analytic continuation

[TABLE]

which in the replica limit simply becomes

[TABLE]

The analytic continuation (19) also provides all the $n$-distances for $n$ odd, which are not given by (17).

In the small interval limit, we can get further results for arbitrary $\Delta\alpha$. In fact, Eq. (14) applies, e.g., for $\alpha=\alpha^{\prime}$ or $\bar{\alpha}=\bar{\alpha}^{\prime}$. In such cases the (unique) quasiprimary field satisfying (12) is $\bar{J}$ or $J$ (respectively), with expectation value in the vertex operator state $|V_{\alpha,\bar{\alpha}}\rangle$ given by $\langle\bar{J}\rangle_{\alpha,\bar{\alpha}}=-2\pi\mathrm{i}\bar{\alpha}/L$ and $\langle J\rangle_{\alpha,\bar{\alpha}}=2\pi\mathrm{i}\alpha/L$. From (14), then, we get

[TABLE]

Here we used $x_{J}=x_{\bar{J}}=1/\pi$ work-td , as follows from (15) together with the calculation of the correlation function of Refs. sierra ; berganza and its analytical continuation in elc-13 . They satisfy the bound (16) with $x_{\rm{max}}(1)=1/\sqrt{6}$.

Another case where (12) applies is the trace distance between vertex operators with $\bar{\alpha}=0$ or $\alpha=0$ and the current states $|J\rangle$, $|\bar{J}\rangle$. For such states, we have $\langle J\rangle_{J}=\langle J\rangle_{\bar{J}}=\langle\bar{J}\rangle_{J}=\langle\bar{J}\rangle_{\bar{J}}=0$. The final result in the short interval limit reads

[TABLE]

The results for some other states will be given in work-td .

All the above results for the compact boson CFT can be checked against numerics in the XX spin chain. We consider a block $A$ with $\ell$ contiguous spins in a periodic chain with $L$ sites. The correspondence between the low-lying states of the spin-chain and the CFT ones is reported, e.g., in berganza ; sierra . As we mentioned, even for these Gaussian states it is not possible to get trace distances in terms of the correlation functions, as instead one can do for the entanglement entropy vidal ; peschel2003 ; afc-09 . However, one can exploit the Gaussian nature of $\rho_{A}$ and $\sigma_{A}$ peschel2003 to access the $2^{\ell}\times 2^{\ell}$ RDM numerically for arbitrary large $L$ vidal ; peschel2003 ; afc-09 , but $\ell$ relatively small, say up to 7 (see work-td for details). Only for even $n$, we can use the techniques of Refs. bb-69 ; fagottiXY to obtain the $n$-distances also for very large $\ell$. Our numerical results for many states are in Figs. 2 and 3. The former shows the trace distance that asymptotically perfectly matches the CFT predictions (i.e. the short-interval expansion for arbitrary states and (20) for the vertex-states with $\Delta\alpha=1$). Fig. 3 reports the $2$- and $3$-distance for some states that perfectly matches available CFT results for arbitrary $\ell/L$.

2D free massless fermion theory.

We now consider a 2D massless free fermion theory, which is a 2D CFT with central charge $c=1/2$, and it is the continuous limit of the critical Ising spin chain. The calculations in the 2D massless free fermion theory and Ising spin chain are parallel to those in the 2D massless free boson theory and XX spin chain. In the CFT, besides the ground state $|0\rangle$, we consider the excited states generated by the primary operators $\sigma$, $\mu$ with conformal weights $(1/16,1/16)$, $\psi$ and $\bar{\psi}$ with conformal weights $(1/2,0)$ and $(0,1/2)$ respectively, and $\varepsilon$ with conformal weights $(1/2,1/2)$.

Making use of the results from Refs. sierra ; berganza ; elc-13 we have that $x_{\varepsilon}$ in Eq. (15) can be analytically calculated $x_{\varepsilon}=1/\pi$ work-td . Using Eq. (14), and the expectation values $\langle\varepsilon\rangle_{0}=\langle\varepsilon\rangle_{\psi}=\langle\varepsilon\rangle_{\bar{\psi}}=\langle\varepsilon\rangle_{\varepsilon}=0,\langle\varepsilon\rangle_{\sigma}=-\langle\varepsilon\rangle_{\mu}=\pi/L$, we get in the short interval limit $D_{1}(\rho_{0},\rho_{\sigma})=D_{1}(\rho_{0},\rho_{\mu})=\ell/(2L)+o(\ell/L)$, $D_{1}(\rho_{\sigma},\rho_{\psi})=D_{1}(\rho_{\sigma},\rho_{\bar{\psi}})=D_{1}(\rho_{\mu},\rho_{\psi})=D_{1}(\rho_{\mu},\rho_{\bar{\psi}})=\ell/(2L)+o(\ell/L)$, $D_{1}(\rho_{\sigma},\rho_{\varepsilon})=D_{1}(\rho_{\mu},\rho_{\varepsilon})=\ell/(2L)+o(\ell/L)$, and $D_{1}(\rho_{\sigma},\rho_{\mu})=\ell/L+o(\ell/L)$. We checked them numerically in the critical Ising spin chain, finding perfect agreement as we will report in work-td .

Conclusions.

In this Letter we developed a replica approach to acess the trace distance in 2D QFT. We exploited our method to provide very general results for the distance between primary states in 2D CFT in particular for short intervals, yielding an explicit form based on the OPE of the twist operators. We also gave explicit results for the free massless compact boson and fermion. We tested analytical CFT results against the numerical trace distances in spin chains finding perfect matches. We only reported here a subset of significant CFT results that we obtained. We will report the calculation details and more examples in work-td , where we will also discuss the consequences of our findings for the relative entropies and fidelities.

Our approach paves the way to systematic studies of trace distances in 2D QFT with several fundamental applications. First of all one can consider different geometries in CFT: open systems, disjoint intervals, finite temperature, inhomogeneous systems, etc. Then, one can study in a CFT after a quantum quench, how the distance between the time-dependent state and the asymptotically thermal state cc-06 shrinks, as well as the difference between distinct statistical ensembles. Massive QFT may be approached adapting the techniques of ccd-08 for the entanglement entropy.

Acknowledgements.

We thank Bin Chen, Song Cheng, and Erik Tonni for helpful discussions. All authors acknowledge support from ERC under Consolidator grant number 771536 (NEMO). Part of this work has been carried out during the workshop “Entanglement in quantum systems” at the Galileo Galilei Institute (GGI) in Florence.