{'fraction_non_alphanumeric': 0.03565020672439348, 'fraction_numerical': 0.00928309540525782, 'mean_word_length': 4.263600903305276, 'pattern_counts': {'":': 0, '<': 0, '<?xml version=': 0, '>': 0, 'https://': 0, 'lorem ipsum': 0, 'www.': 0, 'xml': 0}, 'pii_count': 0, 'substrings_counts': 0, 'word_list_counts': {'cursed_substrings.json': 1, 'profanity_word_list.json': 0, 'sexual_word_list.json': 0, 'zh_pornsignals.json': 0}}
A finite entanglement entropy and the c-theorem

The trace over the degrees of freedom located in a subset of the space transforms the vacuum state into a mixed density matrix with non zero entropy. This is usually called entanglement entropy, and it is known to be divergent in quantum field theory (QFT). However, it is possible to define a finite quantity F(A,B) for two given different subsets A and B which measures the degree of entanglement between their respective degrees of freedom. We show that the function F(A,B) is severely constrained by the Poincare symmetry and the mathematical properties of the entropy. In particular, for one component sets in two dimensional conformal field theories its general form is completely determined. Moreover, it allows to prove an alternative entropic version of the c-theorem for 1+1 dimensional QFT. We propose this well defined quantity as the meaningfull entanglement entropy and comment on possible applications in QFT and the black hole evaporation problem.


Introduction
The density matrix |Ψ Ψ| corresponding to the vacuum state |Ψ can be traced over the degrees of freedom located in a subset of the space giving place to a mixed density matrix with non zero entropy. This is usually called entanglement or geometric entropy. It was argued that this quantity is deeply related to the entropy of black holes [1]. In the black hole spacetime the causal structure provides a natural partition of degrees of freedom, which corresponds to the asymptotic data at infinity and at the horizon respectively. The quantum state relevant for asymptotic observers is obtained by tracing the complete density matrix over the invisible degrees of freedom on the horizon. But |Ψ contains correlations between the field modes inside and outside the black hole, and in consequence, the partial trace leads to a mixed density matrix with non zero entropy. Indeed, several different calculations in specific examples have shown that the geometric entropy is proportional to the area in Minkowski space [1,2,3,4]. More recently the entanglement entropy has been also a subject of much interest in the study of condensed matter systems, specially in relation with the density matrix renormalization group method [5,6].
More generally, the entanglement entropy of the vacuum state can be thought as a special case of a more familiar quantity, the entropy S(V ) contained inside a volume corresponding to a given region V of the space. For gases and other systems this is usually calculated by defining the system in question in the bounded region, what requires the specification of boundary conditions. However, these normally kill the correlations that the global state ρ could present between degrees of freedom in V and its complement −V . To compute S(V ) without artificially modifying the global state ρ we need a partition of the total Hilbert space H as a tensor product of Hilbert spaces inside and outside V , H V ⊗ H −V . Then, the local density matrix is defined by ρ V = T r H −V ρ and its entropy is S(V ) = −T rρ V log ρ V . The local Hilbert spaces H V , density matrices ρ V and entropies S(V ) must Figure 1: (a) The spatial surfaces A and A ′ have the same causal domain of dependence given by the diamond shaped set in this picture. The same entropy should correspond to A and A ′ . Thus, we do not make distinctions between a diamond set and any of its Cauchy surfaces. (b) Two spatial surfaces A and B included in the same global Cauchy surface. Writting area(X) for the d − 1 dimensional volume of the boundary of a d dimensional spatial set X we have area(A)+area(B) = area(A∩B)+area(A∪B).
satisfy certain compatibility conditions that simply express that they arise from a global state ρ and Hilbert space H by partial tracing. Given two non intersecting sets A and B we have that These conditions allow us to use a very important mathematical property of the quantum entropy which is called the strong subadditive inequality (SSA) and which is usefull to relate the entropies corresponding to the different subsystems involved in a tensor product [7,8]. In the present case it acquires the following geometrical form [8,9,10] for any two sets A and B. In addition, the purity of the vacuum state gives the duality relation In Minkowski space the independent degrees of freedom should be assigned to subsets of general Cauchy surfaces and an entanglement entropy must correspond to any of these subsets. Moreover, the causal structure and unitarity imply that this entropy must be the same for different spatial sets having the same causal domain of dependence (see fig.1(a)). It has been shown that the combination of the SSA property, the positivity of the entropy, and the Poincaré invariance of the vacuum state in Minkowski space strongly constrain the function S in any dimensions [10]. The result is that if S is finite for at least one arbitrary set then it has to finite and proportional to the boundary area for any other set, plus a constant term: Here area(A) means the area of the boundary of the spatial surface A and s and α are positive constants. Thus, the area law for the entanglement entropy has its origin in very basic and fundamental properties of relativity and quantum mechanics. In 1 + 1 dimensions the equation corresponding to (4) reads where m A is the number of connected components (or the number of boundary points) of the one dimensional set A. The SSA relation was originally introduced to show the existence of the mean entropy (the limit of entropy divided by volume for large sets) in translational invariant systems [8,9]. We stress that the presence of additional boots symmetries makes the SSA relation a much more powerfull tool. For example, the equation (5) tells that the entropy of a single component set in 1 + 1 dimensions is a constant (if it is finite), while the SSA relation combined with translational symmetry alone only implies that this is a concave function of the length. For different types of sets or more dimensions the contrast is much greater. The equations (4) and (5) apply for finite S. However, all specific calculations, numerical and analytical, have shown that the entanglement entropy is ultraviolet divergent, even for free fields. This divergences can not be softened by adding different matter fields since the entropy is a positive quantity. This indicates that the entanglement entropy may not have a finite covariant meaning in quantum field theory (QFT).
The calculations of S present in the literature have shown that the divergent terms are proportional to the area, which is also suggested by the theorem leading to eq. (4) [10]. Motivated by this fact, we introduce a new quantity constructed out of the function S which is however free from divergences. Let A and B be two spatial sets in Minkowski space which belong to the same Cauchy surface 1 (see fig.1(b)). The symmetric function is finite, since the divergences cancel due to the relation It is also positive because of strong subadditivity and satisfies the duality Besides, F (A, B) has a very suggestive property, not shared by S. When A and B are non intersecting sets F (A, B) is monotonically increasing, From all this, we are lead to propose F as a well defined measure of the degree of entanglement in QFT. In fact, for two non intersecting sets A and B it can be written as where S(ρ 1 | ρ 2 ) = T r(ρ 1 (log(ρ 1 ) − log(ρ 2 )) is known as the relative entropy for two states ρ 1 and ρ 2 acting on the same Hilbert space. This later can be thought as a measure of the statistical distance between a pair of states. In the context of quantum information theory, the particular relative entropy in (10) is called the mutual information between the states ρ A and ρ B in the composite quantum system, and it is used as a measure of the amount of information they have in common [12]. The function F (A, B) for intersecting sets can be defined in terms of the relative entropy for non intersecting ones with the use of additional auxiliary sets. The connection between F and the relative entropy is also satisfying from the mathematical point of view. The origin for the divergence of the standard entanglement entropy can be traced to the impossibility of expressing the Hilbert space H as a tensor product of H V ⊗ H −V in the relativistic case. This partition is unambiguous if the system is defined on a lattice, the local Hilbert spaces being generated by the local degrees of freedom (for example the spin-like operators in a given region).
However, in a relativistic QFT the axiomatic investigations have shown that although there is a well defined notion of local algebras of operators in a volume V (type III Von Neumann algebras in general) there is no Lorentz invariant partition of the total Hilbert space into a tensor product H V ⊗ H −V (see [13,14]). One heuristic reason for this can be seen considering the theory of a free scalar field φ. In the classical theory the phase space attached to a bounded region V is given by initial data φ(x) anḋ φ(x) vanishing outside V . In the quantum case however, only positive energy solutions of the wave equation appear in the annihilation part of the operator φ(x). In momentum space the time derivative is then ǫ p = −i p 2 + m 2 . Now, in real space, the operator given by ǫ p is antilocal, what means that it transforms any function vanishing outside an open set V in a function which does not vanish identically in any open subset outside V [14]. This implies that one can not have 0|φ(x)|ψ and 0|φ(x)|ψ vanishing simultaneously in the same region of space, where |ψ is any one particle state. In general the moral is that in QFT there is no covariant meaning for the localization of states, and what can be unambiguously localized are the field operator algebras. In this sense it is remarkable that even if a notion of entropy for a state in a given algebra may not exist (type III algebras do not contain a trace), the relative entropy of two states for the same Von Neumann algebra has a well defined mathematical meaning [15].

Entanglement entropy in 1 + 1 dimensions
The equation (6) implies the following relation between the finite F functions for any A, B and C. In a given regularization scheme, as S goes to infinity these relations between finite quantities are maintained. The most general form of a function that solves (11) in 1 + 1 dimensions can be found by a long but straightforward calculation that we are not presenting here. It follows that Evidently, this equation has the same form as (6) but now the one set function G is perfectly finite.
Since the meaningfull quantity is F , the function G(A) is defined up to an arbitrary term proportional to the number m A of connected components in A. Thus, for the one component sets there is a "gauge" symmetry associated to an additive constant. The positivity of F implies strong subadditivity for G, and from (8) The crucial difference between G and an entropy is that it can attain negative values. This must be so if G has some dependence on the size of the sets, because otherwise, as we have already mentioned, eq. (5) would apply for G. Moreover, it must attain negative values with arbitrarily big modulus. If not, it could be converted into a positive function by adding a suitable term proportional to m A .

Entanglement entropy in Conformal Field Theory
For the special case of a conformal field theory (CFT) and when the sets A and B are one component and intersecting, the eq. (12) allows us to obtain the general form of F (A, B). We see from figure 2(a) that only four points determine the position of the diamonds corresponding to A and B. As F (A, B) must be invariant under global conformal transformations, general results ensure that it must be a function of the cross ratios with where we have written u ij = u i − u j and v ij = v i − v j and the (u i , v i ) are the null coordinates of the point x i . On the other hand, for one component sets, G can be written as a function of the length of the diamond base r ij = ( Using this and equations (12) and (14) we get the general form for G and F G(A) = k log(r A ) + β .
where k and β are constants, with k ≥ 0.
The conformal symmetry provides a simple argument in order to explain why F is finite while S is not. Both quantities are supposed to be invariant under global conformal transformations which leave the vacuum invariant, but while F is a function of four points only two points determine the argument of S for one component sets, and there is no possibility of forming a cross ratio with two points. Thus S must be either infinite or a constant.
Several authors have calculated the entanglement entropy S in 1 + 1 conformal field theories with different regularization prescriptions, both numerically and analytically [2,4,5,16]. The result is S = (1/6)(c +c) log(r A /ǫ), where ǫ is an ultraviolet cutoff, and c andc are the holomorphic and antiholomorphic central charges. This formula can not be used for l A ≤ ǫ that gives S ≤ 0. According to equation (6), our results (16) and (17), obtained from very general considerations, are perfectly consistent with this expression for S, identifying k with (c +c)/6. Thus, G can be interpreted as a regularized entropy, G(A) = k log(r A µ), with µ a renormalization scale. The fact that G is negative in some range causes no problem since its physical meaning is only up to a constant term.
From eq. (17) we see that the divergences appear in F reduced to certain special configurations of the diamonds. This is when r A∩B goes to zero, which is not surprising, since in that limit the two diamonds separate each other and F turns into a different function, the one for non intersecting one component diamonds we discuss below.

An entropic c-theorem
Now we look for the general form of G(A) ≡ G(r A ) for one component sets in 1 + 1 dimensional theories. Consider two one component sets A and B of the same size r 1 , intersecting in a segment of size r 1 − r 2 with r 2 ≤ r 1 . It follows from (13) applied to A and −B that Thus, G(r) is increasing and G ′ ≥ 0. The SSA relation for intersecting diamonds disposed as shown in the figure 2 It can be shown that all other inequalities coming from SSA for two intersecting one component diamonds are less constraining than this relation. The meaning of (19) becomes more clear defining the such that the domain ofḠ is the whole real line. Equation (19) becomes This relation is called weak concavity, and it is known to be a property of the entropy for translational invariant systems in the original length variable. Here we have it in the logarithmic variables. Using repeatedly this equation we can prove concavity forḠ, that is for any λ ∈ [0, 1]. The concavity ofḠ can be more simply writtenḠ ′′ ≤ 0. Introducing a new function C(r) ≡ r G ′ (r) we summarize all the constrains on the original function G as According to the equations (23) and (24) the dimensionless function C must be positive and decreasing with r. Since it depends on G ′ it is also a physically meaningfull quantity independent of the ultraviolet cutoff. Thus, the renormalization group equation for C reads where τ is the substraction point, the g i are the different dimensionless coupling constants and β i (g) the corresponding beta functions. This equation expresses that the total derivative of C with respect to τ is zero, what follows from the fact that C is an observable quantity in a renormalizable theory. Note that in consequence, the anomalous dimension term is not present in (25). By dimensional analysis C has to be a funtion of (τ r) and the dimensionless coupling constants, then we have As C is decreasing with r we see from eq. (25) and (26) that C(r 0 , g) for fixed r 0 is a function of the coupling constants which decreases along the renormalization group trajectory. Moreover, at the fixed points, corresponding to conformal field theories, eq. (16) implies that C(r 0 , g) is a constant k = (c +c)/6, stationary under the renormalization group flow. This is in fact the statement of the Zamolodchikov theorem [17].
Remarkably, this theorem follows here from the properties of the entropy and the Poincaré symmetry without resorting to quantum fields. Also, the unitarity and causality of the theory are implicitly used in the fact that the entropy of a given set does not depend on the particular choice of the Cauchy surface, what is crucial for the arguments that lead to eq. (19) (see figure 2(b)). Moreover, the SSA property requires a self-adjoint and positive density matrix which is also related to unitarity (however, it also works for classical probability distributions) [7,8].
The C charge in eq. (23) has an interesting physical meaning: it measures the variation of the geometric entropy with the size of the set whose degrees of freedom are traced over. For example, for massive fields, the entropy saturates at a given radius (see for example [5]), what leads to the vanishing of C for large r. This is in accord with the renormalization group flow interpretation of the running of C given by eq. (26) since at the infrared no available degrees of freedom remain in the massive case.
In relation with the massive C function we make the following remark that gives additional support to the connection of the entropy F with the algebraic approach to QFT. Numerically we find that the C function (23) for a free scalar field of mass M decreases exponentially, C(r) ∼ e − √ 3M r , for large r, what also happens for the Zamolodchikov c function. Adding independent scalar fields we have a contribution to C(r) due to the sum of the exponential tails which is of the form dM σ(M )e − √ 3M r , where σ(M ) is the density of fields per unit mass. We can choose an exponentially increasing density T H in such a way that the theory has a maximal temperature T H (Hagedorn temperature). In this case the divergence of G does not take place at r = 0 but at a finite distance r ∼ T −1 H . This coincides with the results of [18] which tell that a consistent tensor product structure can not be given to the states on the algebras of two non intersecting sets when their separation distance is less than some constant times T −1 H . Some relations between the geometric entropy and the renormalization group flow were already suggested in the literature based on numerical results [5]. Moreover, interesting entropic c-theorems were introduced in [19]. These also rely on the properties of the entropy. However, they do not involve the entanglement entropy between the degrees of freedom in different regions of the space but the relative entropy between the vacuum states corresponding to different values of the theory couplings.
The renormalization group flow of the Zamolodchikov c function is given in terms of the energy momentum tensor correlators. It is likely that the energy momentum tensor is also involved in the running of the entropic function C proposed in this paper. This would be very interesting, specially taking into account that one of the originals aims of the investigations about the geometric entropy was the underestanding of the relation between entropy and gravity.

The two component set function
The equations (23) and (24) give the most general form of the function F (A, B) in 1 + 1 dimensions for intersecting one component sets A and B. Of course, these leave a lot of freedom, but this must be so, since F contains information on the mass spectrum of the theory. The analysis can be continued considering the multicomponent set functions, that is, the case in which the sets A and B are multicomponent or non intersecting. Then, the function F and the relevant inequalities involve the function G evaluated on multicomponent sets. The general analysis is outside of the scope of this letter. Here we show only some constrains for the simple case of two non intersecting one component sets A and B lying in a single spatial line in a CFT. These sets are as before determined by the position of their four edge points, what implies due to global conformal invariance that F is a function of the cross ratio where r A and r B are the sizes of A and B and r C is their separating distance. We can rewrite eq. (27) as with U (η) = F (η) + k log(1 − η). The duality (8) leads to Besides, from the SSA relation between A ∪ B and another set C with one or two components it follows that These inequalities highly constrain the function U , and in particular show that it has to be bounded in its domain η ∈ [0, 1]. Thus, the only singular points in G(A ∪ B) come from the first term in the right hand side of (29). In particular in the limit B → −A, r C = ǫ → 0 we get F → 2k log(r A /ǫ). From eq. (6) this gives consistent with previous calculations [16].
We have checked numerically the formula (29) for a Majorana and a Dirac fermion (c = 1/2 and c = 1 respectively) using the methods of [5,20]. The result is U ≡ 0 and k = 1/6 and k = 1/3 respectively. On the other hand, we have also considered the theory of a free massless boson (c = 1). The existence of a zero mode provides an additional infrared divergence to the entanglement entropy which is also present in F (this happens for all theories with non compact global symmetry groups). To regularize it we have introduced a small mass M and attached the theory to a cylinder of circumference L such that M L ≪ 1. In this case the numerical result is where is the expression of η in the cylinder. With r A , r B , r C ≪ L one recovers η cyl → η. The formula (35) satisfies the inequalities (31-33) with k = 1/3, except when η (M L) (9/2) or (1 − η) (M L) (9/2) where the mass enters into the game and equation (35) and the conformal symmetry do not hold any more. This is why (35) does not seem to lead to a bounded U . The point we want to make here is that the function U has the ability to distinguish between different models with the same central charge (c ≥ 1).

Final remarks
One could wonder if the whole set of entanglement entropies are in one to one correspondence with the different QFT. In other words, is it possible to uniquely define a QFT by the set of its entanglement entropies?. This is likely, since the local algebras of all QFT are the same mathematical objects, independent of the theory and the space-time dimension [13]. Thus, the way they are entangled to each other must play a central role. If one accepts this, a second question naturally appears: is it the = const. Further interest to these questions is given by the fact that the entanglement entropy F has a nice property suited to study dimensional reduction. Take for example the sets of the form A × [x] in d + 1 spacial dimensions, where [x] is an interval of length x and A is any d dimensional set. Then the functionF is well defined and must satisfy all requirements of an F function in d dimensions [10]. Generalizations of the results of this paper to higher dimensions using this construction are currently under investigation. Finally, we suggest an interpretation of F in the black hole evaporation problem. Take A as the Rindler wedge and let B be a diamond outside A as shown in fig. 3. Then F (A, B) can be interpreted, at least in certain limit, as the amount of entropy from the Unruh thermal radiation that an observer can detect in an experiment running for a finite period of time corresponding to the set B (see related ideas in [4,21]). This period measured in the boost parameter ν = arcth(t/x) is ∆ν = log r B + r C r C .
Now, the equations (27) and (29) for r A → ∞ give Thus, as U is bounded, for big enough ∆ν this gives F (A, B) ≃ k∆ν. We also have ∆ν = a∆τ , where τ is the proper time meassured by an accelerated observer with constant acceleration a. This formula tells that the entropy is proportional to the diamond time ∆τ times a constant flux of entropy ka due to a constant flux of Unruh radiation. Indeed, the Unruh temperature is T = a/(2π) and in the high temperature limit (adequate to the limit taken above) the flux of entropy per unit time in a CFT has a universal expression given by ∆s/∆τ = π c+c 3 T [22]. Therefore, the identification of F with the total entropy flux during the interval ∆τ lead us again to the equation k = c+c 6 . In the black hole case ∆ν should be interpreted as ∆τ /(4M BH ), where τ is the time as measured by the asymptotic observers and M BH is the black hole mass. Thus, F would be proportional to the asymptotic time, corresponding to a constant flux of Hawking radiation. For a real black hole the back-reaction must be included. In four dimensions the black hole lifetime is ∆τ ∼ M 3 BH , giving place to a maximal observable entropy F (A, B) ∼ M 2 BH , which is proportional to the horizon area.

Acknowledgments
H.C. thanks the invitation to visit the ICTP where this work has been done.
Note added.-After the submission of this paper to the arXiv data-base, the reference [23] appeared, showing a calculation of the multi-set CFT entropy functions. Their general results are in agreement with the particular cases considered in Sections 2.A and 2.C.

Erratum:
1.-Equation (7) eliminates the divergences in F (A, B) only in two dimensions. In more dimensions additional subleading terms are present and F (A, B) does not converge for generic A and B. 2.-In Section 2.B the long distance behaviour C(r) ∼ e − √ 3M r should read C(r) ∼ e −2M r . 3.-In Section 3 the large ∆ν limit is the low (rather than high) temperature limit. There is a factor two in ∆s/∆τ which should read π c+c 6 T . This means that F represents twice the total entropy flux during the time ∆τ .