Relative entropy of coherent states on general CCR algebras

For a subalgebra of a generic CCR algebra, we consider the relative entropy between a general (not necessarily pure) quasifree state and a coherent excitation thereof. We give a unified formula for this entropy in terms of single-particle modular data. Further, we investigate changes of the relative entropy along subalgebras arising from an increasing family of symplectic subspaces; here convexity of the entropy (as usually considered for the Quantum Null Energy Condition) is replaced with lower estimates for the second derivative, composed of"bulk terms"and"boundary terms". Our main assumption is that the subspaces are in differential modular position, a regularity condition that generalizes the usual notion of half-sided modular inclusions. We illustrate our results in relevant examples, including thermal states for the conformal $U(1)$-current.


Introduction
Entropy and related correlation measures are of fundamental importance in quantum physics; not only in information theory, but also in thermodynamics and quantum field theory.
Mathematically, the most appropriate generalization of the classical notion of (relative) entropy to quantum systems, or noncommutative probability spaces, is formulated in terms of normal states on von Neumann algebras [Ara76] (see also [OP04,BFS16]). However, while the formalism is quite easy to handle for type I factors, where normal states are described by positive trace-class operators and the entropy can be computed by means of traces, applications to the type III 1 factors occurring generically in quantum field theory [BDF87] require working with (relative) Tomita-Takesaki modular objects, which are difficult to decribe explicitly in examples.
Recent work in quantum field theory [LX18,Lon20] has focussed on entropy measures for algebras associated with certain subregions of spacetime, and the dependence of the entropy of a given state depending on the spacetime region. Specifically, one considers the relative entropy between a ground state and a coherent excitation in the setting of linear fields [CGP19,CLR19] or related situations in chiral conformal quantum field theories [Hol20,Pan20,Pan21]; in some geometric situations, specific information about the (relative) modular operator is available here and allows for explicit results.
Let us illustrate the situation in an example, following [CLR19]. Consider a massive free field in 3+1dimensional Minkowski space, given in terms of the well-known symplectic space (K, σ) and real subspaces L(O) ⊂ K associated with space-time regions O, and the corresponding Weyl (CCR) algebras A(O). Further let ω be the vacuum state on these algebras, and consider a coherent state ω g = ω(W (g) * · W (g)), where g ∈ K and W (g) is the corresponding Weyl operator. Consider the standard left wedge W = {x : x 1 < 0, |x 0 | < |x 1 |} ⊂ R 4 , and for t ∈ R the shifted region 1 W t = W + (t, t, 0, 0). Then the relative entropy between ω g and ω with respect to the algebra A(W t ) can be computed as [CLR19] S A(Wt) (ω g ω) = 2π where T µν g is the single-particle stress-energy tensor of the wave function g. Consequently, with v = (1, 1, 0, 0), d dt S A(Wt) (ω g ω) = 2π x 1 <t dx v µ T 0µ g (t, x) ≥ 0, (1.2) d 2 dt 2 S A(Wt) (ω g ω) = 2π The second derivative is nonnegative, and hence the relative entropy is a convex function of t; this can be regarded [CF18] as a variant of the Quantum Null Energy Condition (QNEC). More generally, the QNEC is understood as a relation between certain expectation value of the energy density and the second derivative of the relative entropy [BFK + 16], which is also suggested by Eq. (1.3). In this paper, we will only investigate derivatives of the entropy along a family of regions or subspaces, but will not comment on the relation with the energy density.
Apart from convexity, one may observe that the first derivative (1.2) is given by a "bulk term" (an integral over a Cauchy surface for the wedge region) while the second derivative (1.3) is given by a "boundary term" (an integral over the edge of the wedge at x 1 = x 0 = t).
This motivates the question which of these observations are a coincidence of the specific system chosen, and which of them generalize to a wider context.
In this paper, we ask such questions in a generic setting. We remain within the context of CCR algebras, i.e., the algebras in question are still generated by the "second quantization functor" from a symplectic space K and certain real subspaces L ⊂ K; and our states will be of the quasifree type. However, we abstract from the specifics of the above example.
As a first point, we investigate the connection between the symplectic (single-particle) structure and the relative entropy on the CCR algebras. Essentially, the methods of [CLR19] apply whenever the symplectic subspace L ⊂ K above is standard and factorial, and the state ω is quasifree and pure. (These notions will be recalled in Sec. 2.) However, in applications in physics, also non-pure quasifree states are of importance, for example thermal states [RST70,BR81] or Hadamard states in quantum field theory on curved spacetimes [KW91,Rad96]. Moreover, while factorial subspaces are usual in quantum field theory, they are certainly not the most general case (cf. [Ver97]).
We aim to prove a unified formula for the relative entropy between a quasifree state ω and an associated "coherent excitation" ω g in the general case. Our approach is as follows. We start with a generic symplectic space and consider the CCR algebra over it, equipped with a quasifree state. The state is not assumed to be pure; rather, using the well-known purification construction [Wor72,KW91], we extend it to a pure state on a larger algebra. Now given a closed subspace L, we decompose the extended space (and the corresponding CCR algebra) into factorial, abelian and nonseparating parts, and compute the relative entropy for these. We give a unified formula for the relative entropy between coherent states with respect to A(L), where L is a generic subspace, in terms of the modular data associated with L.
Second, we consider a family of subspaces {L t }, depending on a real parameter t, in particular when L t increases with t; we ask how the relative entropy S t (g) = S A(Lt) (ω g ω) for given g ∈ K changes with t.
To this end, the following technical insight is important. With each subspace L s one obtains, as in [CLR19], a projector Q s which projects onto the "L s -entropy relevant part" of K (in the factorial case, onto L s itself) and annihilates the symplectic complement L ′ s . However, this projector is unbounded in the usual topology of the symplectic space K; even more, its domain will usually depend on the parameter s, which makes it particularly challenging to analyze a change in the parameter. However, let us equip the space with an (indefinite) scalar product arising from the semipositive quadratic form S t (g), where t = s in general. With respect to this Hilbert space structure, it turns out in relevant cases that the projector Q s is orthogonal, in particular bounded. We say in this case that the spaces L s , L t are in differential modular position, a condition that underlies our analysis, and resembles the concept of geometric modular action (see [Bor00]).
This structure then allows for the desired analysis of bulk vs. boundary terms: For fixed g ∈ K, let us consider the function T g (s, t) = S t (Q s g), which equals the entropy on the diagonal t = s. A change in s near the diagonal then corresponds to an abstract "boundary change" while a change in t corresponds to a "bulk change". Analyzing the monotonicity properties of T g , we establish estimates between the partial derivatives of T g (at s = t − 0) and the desired derivatives of the entropy.
We note that convexity of S t cannot be expected in such a general setting; it is already not preserved under a smooth reparametrization of the family of spaces, which our definition admits. However, we establish lower estimates on the second derivative (in the sense of distributions) that replace convexity. Also, the observation from above that the first derivative contains only bulk terms, while the second derivative contains only boundary terms, does not hold up in general, and is replaced by a more nuanced picture.
We verify the regularity condition of "differential modular position" in a number of examples, mainly but not exclusively from quantum field theory. In particular, it turns out that in half-sided modular inclusions of symplectic subspaces (cf. [Bor00,Lon07]), our condition is always fulfilled. Also, we treat relative entropies for halfline algebras in the conformal U (1)-current in thermal states, which to our knowledge have not appeared in the literature.
The paper is organized as follows: Sec. 2 defines our setting, recalls the purification and decomposition construction for symplectic spaces, and establishes the unified formula for relative entropies in terms of single-particle objects. In Sec. 3, we investigate the relative positions of several subspaces, in particular one-parameter families of inclusions; we formulate our main condition (differential modular position) and derive estimates for the second derivative of the relative entropy. Then we show that all half-sided modular inclusions fit into our framework (Sec. 4). In Sec. 5 we give examples from quantum mechanics, quantum field theory and classical probability theory in which our framework is applicable, illustrating various cases that can occur with respect to the derivative estimates we established. We end with a conclusion and outlook in Sec. 6. The appendix recalls definition and fundamental properties of the relative entropy on C * -and von Neumann algebras.

Entropies in nonpure states
We first introduce our setting of symplectic spaces, purification and the decomposition of subspaces in Sec. 2.1. Then (Sec. 2.2) we pass to the associated CCR algebras and their decomposition, and express the relative entropy between coherent states in terms of the single-particle modular data. Sec. 2.3 establishes some approximation properties needed in later sections.

Single-particle structure
The basic object we work with is as follows: Definition 2.1. Let K be a vector space over R and τ, σ two bilinear forms on K. The triple (K, τ, σ) is called a symplectic Hilbert space if (K, τ ) is a separable Hilbert space, (K, σ) is a symplectic space, and if ∀f, g ∈ K : σ(f, g) 2 ≤ τ (f, f )τ (g, g). (2.1) Here σ is allowed to be degenerate as a symplectic form; we can (and will) assume without loss of generality that the dimension of its kernel is either even or infinite. (Otherwise consider the direct sum of K with a one-dimensional space, on which σ is set to vanish.) Note that K is assumed a priori to be complete with respect to τ -convergence; in applications one often starts with a pre-Hilbert space in the first step, and then takes its completion, but note that e.g. a non-degenerate form σ on the non-completed space might be degenerate on the completion (cf. [Ver97]).
If K is a Hilbert space over C with complex scalar product · , · , then a standard example for Definition 2.1 is τ (f, g) = Re f, g and σ(f, g) = Im f, g . In fact, this is exactly the case when the quasifree state induced by τ on the CCR algebra over (K, σ) (see Sec. 2.2 below) is a pure state [MV68]; hence we will call (K, τ, σ) pure in this case. In general, it is always possible to embed (K, τ, σ) into a pure symplectic Hilbert space (K ⊕ , τ ⊕ , σ ⊕ ), i.e., such that τ ⊕ , σ ⊕ are extensions of τ , σ. This construction is known as purification, and we will present it here in the form of [Pet90,Ch. 4]; see also [KW91,Appendix A].
Due to (2.1), we can write σ = τ ( · , D · ) with an operator D, where D ≤ 1. Using the polar decomposition of D on the orthogonal complement of ker D, and a suitable choice 2 on ker D, we obtain two bounded operators C, |D| such that (2.2) (We denote the adjoint with respect to τ by †, whereas we will denote adjoints on complex Hilbert spaces by * later on.) We now define the space K ⊕ := K ⊕ K, which is a vector space over C with respect to the complex structure given by the operator In fact, defining the bilinear forms (f, g ∈ K ⊕ ) K becomes a complex Hilbert space with the scalar product · , · ⊕ , and a nondegenerate symplectic space with symplectic form σ ⊕ . Identifying K with K ⊕ 0, the restrictions of τ ⊕ and σ ⊕ to K × K are τ and σ respectively, as the notation suggests. Now let L ⊂ K be a closed subspace. (Note that closure in K-norm is crucial for the following.) We decompose L in a standard way (cf. [Hal69]) as follows: We set where L ′ denotes the symplectic complement of L. The spaces L f , L a , and L ∞ are called the factorial, abelian and nonseparating parts of L, respectively, for reasons that will become clear below. We then have: Lemma 2.2. K ⊕ is isomorphic to the orthogonal direct sum and under this isomorphism (2.14) Proof. One shows by direct computation that L a is complex-orthogonal to L ∞ ; also, L a is real-orthogonal to ı ⊕ L a , hence L ⊕ a is closed. The other parts follow directly from the definitions (2.7)-(2.12). All three components of L may be present in general: in quantum field theory, one usually considers purely factorial subspaces, i.e., L = L f (see Examples 5.3 and 5.11); but in other situations, L may be purely abelian (L = L a , Example 5.12), or one may have L = L ∞ (part of Example 5.1), and of course direct sums of these can be formed. We note some special cases: Remark 2.3. If (K, τ, σ) is a pure symplectic Hilbert space, then D = −i, hence ı ⊕ acts by the diagonal matrix i 0 0 −i . In the decomposition of Lemma 2.2, this leads to 0 ⊕ K ⊂ L ⊕ 0 , and all other spaces L f , L a , L ∞ etc. being contained in K ⊕ 0. In this sense, if (K, τ, σ) is already pure, we can ignore the purification construction.
Remark 2.4. If specifically K = L in Remark 2.3, then L ∞ = K ⊕ 0, L f = L a = {0}, L ⊕ 0 = 0 ⊕ K. Remark 2.5. For a symplectic Hilbert space (K, τ, 0) (i.e., for σ = 0), even-or infinite-dimensional, we where ⊥ denotes the orthogonal complement in K. In the following, we shall denote the complex-linear orthogonal projectors onto L ⊕ f etc. as P ⊕ f etc. We also denote by P a the real-orthogonal projector onto L a , and by P f the real-linear projector with image L f and kernel L ′ f . Note that P f is not bounded (or orthogonal) in general, but closed on its domain We also consider the subspaces L s : Hence [RvD77] we obtain Tomita-Takesaki objects J L , ∆ L with respect to this subspace. We set K L := − log ∆ L , then extend this operator K L by 0 to L ⊕ 0 and consider it as undefined on L ⊕ ∞ \{0}. We denote the modular group by U L (x) = exp(−ı ⊕ xK L ), again defined on L ⊕ 0 ⊕ L ⊕ s . It is important in the following that the projector P f can be written as a function of the modular objects: Lemma 2.6. ([CLR19, Theorem 2.2]) Let a(λ) = (1 − λ) −1 , b(λ) = λ 1/2 a(λ). Then For use in future sections, we also consider the closed, real-linear projector (2.16) Note that img Q L = L in the purely factorial case (L = L f ), but in general img Q L = L; rather, as will become clear in the next subsection, Q L projects onto the "entropy-relevant part" of the space. (See Lemma 2.12(v) and Theorem 2.13 in particular.) However, we always have ker Q L = L ′ . In other words, img Q L = (ker Q L ) ′ in general. We also note: Lemma 2.7. For 0 < ǫ < 1, let Q (ǫ) be the spectral projector of log ∆ L for the set Then D (0) is a core for Q L , and D (0) ∩ L ⊕ s a common core for ∆ L and log ∆ L .
Proof. We can suppose without loss of generality that we are in the factorial case, i.e., L = L f , since on L ⊕ a we have that ∆ L ↾ L ⊕ a = 1, log ∆ L ↾ L ⊕ a = 0, and Q L ↾ L ⊕ a is bounded, while on L ⊕ 0 and L ⊕ ∞ the statement is clearly trivial. That D (0) ∩ L ⊕ s is a common core for ∆ L and log ∆ L is immediate by functional calculus. That D (0) is a core for Q L in the factorial case follows by the expression of Q L in terms of ∆ L and J L given in Lemma 2.6.
On A K , the bilinear form τ induces the quasifree state 3 ω by (2.18) we use the same notation for its extension by τ ⊕ to A ⊕ K and the restrictions to subalgebras, suppressing the dependence on τ where no confusion can arise. Related to ω, for each g ∈ K we consider the coherent state 4 ω g = ω(W (g) * · W (g)); (2.19) note that ω 0 = ω. We are interested in the relative entropy between the ω g (for different g) as states on the C * -algebra A L ; see Appendix A for a brief review of this concept. As a first step, we remark that the relative entropy respects the decomposition of L: Proposition 2.8. Let (K, τ, σ) be a symplectic Hilbert space. For any closed subspace L ⊂ K, we have (2.20) Proof. Due to Lemma 2.2, and noting that the pure quasifree states are faithful on the respective subalgebras, we know that A ⊕ K is isomorphic to the (spatial) tensor product of C * -algebras and under this isomorphism and ω decomposes in the same way. This decomposition holds analogously for the induced von Neumann algebras in the GNS representation of A ⊕ K associated with ω. Thus, due to additivity of the relative entropy in this situation (see Lemma A.2 in the appendix), we obtain (2.20). (This includes the obvious observation that the summand with respect to L ⊕ 0 vanishes.) 3 also known in the literature as a quasifree state with vanishing one-point function 4 An alternative nomenclature is quasifree state with nonvanishing one-point function.
We will now compute the three terms in (2.20) individually. We start with the abelian part, following standard methods (cf. [VS11]).
Proposition 2.9. For any g ∈ L ⊕ a , where P a is the (real-linear) projector onto L a .
Proof. Since K is separable, the von Neumann envelope of A L is generated by the algebras for finitedimensional subspaces of L. Lemma A.1 in the appendix shows that S Aa (ω g ω) is determined by the supremum of the entropy for these subalgebras; hence it suffices to prove the statement for the case of finite-dimensional L ⊕ a . Also, on the algebra A a , the state ω g coincides with ωĝ whereĝ = (1 − P a )g; hence we can assume without loss that g ∈ (1 − P a )L ⊕ a = ı ⊕ L a . In this case, after a suitable choice of basis, L ⊕ a with the scalar product ·, · ⊕ can be identified with C n and its standard scalar product, with the real subspace R n corresponding to L a . The GNS representation π for (A a , ω) acts on L 2 (R n , dµ) where dµ = (2π) −n/2 exp(− x 2 /2)d n x, with π(W (f )) being multiplication with exp i f, · , and π(A a ) ′′ = L ∞ (R n , dµ). The states ω and ω g are vector states with vectors Ω(x) = 1, ). The relative modular group turns out to act by multiplication with exp(−2it ı ⊕ g, x + 2it( g ⊕ ) 2 ). The relative entropy can then be computed from the general definition (A.1), which yields the result (2.24).
Of course, this relative entropy coincides with the usual Kullback-Leibler divergence of Gaussian distributions (cf. [OP04,p. 81]). In the proof, we have used our simplifying assumption that K is separable, but by methods of the theory of Gaussian fields [VS11], we expect that this assumption is actually dispensable.
Next, we consider the factorial part, for which the relative entropy is known from [CLR19].
Proof. We sketch the relevant techniques from [CLR19]. Since (L ⊕ f , τ ⊕ , σ ⊕ ) is pure, the GNS representation π of (A f , ω) acts on the Fock space over L ⊕ f , and in that representation both ω and ω g are vector states: ω corresponds to the Fock vacuum vector Ω, and ω g to the vector Ω g := π(W (g))Ω. The vector Ω is cyclic and separating for π(A f ) ′′ , and the associated Tomita-Takesaki modular group is ∆ it (2.26) With the Weyl relations (2.17) and ∆ it Therefore the relative entropy is (2.28) Hence (2.25) holds for g ∈ L f ∩ dom K L . It also holds for g ∈ L ′ f ∩ dom K L , since in that case both sides of the equation vanish. The result for general g ∈ L ⊕ f ∩ dom K L follows by a density argument that employs Lemma 2.6; see [CLR19,Sec. 4.4].
On the nonseparating part, one finds the relative entropy as follows: Proposition 2.11. For any g ∈ L ⊕ ∞ , Ch. 4] and ω and ω g are given by vector states Ω and Ψ := π(W (g))Ω there. The support projections of these states are hence the projectors P Ω and P Ψ respectively; and P Ω ≤ P Ψ if and only if they are equal, i.e., for g = 0. The statement then follows from the definition of the relative entropy, see the appendix.
Our goal is now to establish a unified formula that applies to all these cases, linking the relative entropy on the CCR algebras to a quadratic form at single-particle level. To that end: (2.30) extended by zero to L ⊕ 0 and undefined on L ⊕ ∞ \{0}. (The function c is extended by continuity to λ = 0.) Then: (i) There is a unique closed real-linear quadratic form S L associated with R L , which is positive; Proof. Since (1 − J L )/2 is a real-orthogonal projector, it is clear that R L is positive. Thus R L has a unique positive closed quadratic form associated with it, showing (i). Further, one computes on L ⊕ s , and since λ → c(λ)c(−λ) is bounded by 1, (ii) follows, also on L ⊕ 0 . Consequently, the form domain of S L is the same as the operator domain of c(K L ); since c(λ) → 0 as λ → −∞ and c(λ) ∼ λ 1/2 as λ → ∞, it can be written as in (iii). We prove (iv) separately for the restrictions to L ⊕ a and L ⊕ f ; it is trivial on L ⊕ 0 . Now on L ⊕ a , the statement follows from c(0) = 1, while on L ⊕ f , one computes ker S L = ker P f by Lemma 2.6, and We will sometimes write S L (f ) as shorthand for S L (f, f ). We are now ready to state the main result of the section: Theorem 2.13. For any f, g ∈ K ⊕ , we have and (2.32) follows for all g ∈ L ⊕ f ∩ D (0) from Proposition 2.10. Using approximation techniques [CLR19, Theorem 4.5], the relation can be extended to all g ∈ L ⊕ f , including the case where the two sides of (2.32) are infinite. Now consider g ∈ L ⊕ a . We note that L ⊕ a = ker log ∆ L and c(0) = 1, hence R L acts as 1 − J L = 2(1 − P a ) on L ⊕ a . Thus the proposed result (2.32) holds for g ∈ L ⊕ a , see Proposition 2.9. Likewise, Proposition 2.11 shows that (2.32) holds for g ∈ L ⊕ ∞ , with both sides being infinite unless g = 0. Applying Proposition 2.8 now concludes the proof.

Approximation properties
For the following, we establish some approximation properties for the entropy form and the modular group. Apart from the Hilbert space norm given by τ on K (and extended to · ⊕ on K ⊕ ), we consider the following norms on K ⊕ or subsets of it: It is clear that the K L -graph norm is stronger than the S L -graph norm, which is in turn stronger than the seminorm · L . We denote the closure of dom S L in · L , modulo the kernel L ′ of the seminorm, as X L ; for formal reasons we explicitly denote the isometric inclusion of (dom S L , S L ) into X L as ϕ L . Then X L becomes a Hilbert space with the (continuous extension of) the scalar product ϕ L f, ϕ L g L = S L (f, g).
Lemma 2.14. The modular group U L maps dom S L into dom S L , and this action is strongly continuous in the S L -graph norm.
where Lemma 2.12(ii) was used. This vanishes as s → 0 due to strong continuity of U L in the K ⊕ -norm.
The following lemmas for a fixed closed subspace L ⊂ K will allow us to identify X L with a "concrete" Hilbert space in examples.
Proof. Let ε > 0 and Q (ε) be as in Lemma 2.7. Then for any v ∈ K ⊕ , by Lemma 2.7 we have Q (ε) v ∈ dom Q L . Also, for any v ∈ dom(S L ), by the expression for the relative entropy in Theorem 2.13, we have Q (ε) v → v in S L -graph norm as ε → 0. Furthermore for v ∈ dom(S L ), by functional calculus, as ε → 0.-If here L = L f , one has img Q L = L and the second statement follows.
Lemma 2.16. Let D ⊂ L be a core for the generator of the strongly continuous (with respect to the norm Proof. In this proof, we drop the index L on K L . Note that by functional calculus, the norm induced by the positive self-adjoint operator c(K) 2 + c(−K) 2 , where λ → c(λ) is as in Lemma 2.12, is equivalent to the norm induced by 1 + |K|, while the graph norm of ı ⊕ K ↾ L is induced by 1 + K 2 and thus stronger. Hence since D is a core for ı ⊕ K ↾ L, it is also dense in L ∩ dom K in the norm induced by c(K) 2 + c(−K) 2 and consequently, by Lemma 2.12(i)-(ii), dense in the S L -graph norm.

Entropies for subspaces
We will now consider several subspaces L t ⊂ K, and relations between the entropies related to them. To simplify notation, we will usually denote the related objects as S t , ∆ t , etc. rather than S Lt , ∆ Lt etc.

Two subspaces
We begin with the relation between two subspaces, say, L 0 and L 1 , and their associated entropy forms. Let us first mention: Proof. This follows from Theorem 2.13, since the relative entropy is known to increase with the algebra considered (Lemma A.3).
We now investigate the relation between the projector Q 0 (on the "entropy relevant part" for S 0 ) and the entropy S 1 . Heuristically, we expect in relevant cases that in other words, that the projector Q 0 is "orthogonal" with respect to the bilinear form S 1 . However, the relation (3.1) needs to be read with care, as in general neither domain nor image of Q 0 will consist only of vectors of finite entropy S 1 . The precise version of our condition is given as: Definition 3.2. Let L 0 and L 1 be closed subspaces of a symplectic Hilbert space (K, τ , σ). Define We say that the pair (L 0 , L 1 ) is in differential modular position if This condition may seem restrictive, but it is in fact fulfilled in many relevant examples: in the conformal U (1)-current for half-line algebras, both in the vacuum (Example 5.3) and in KMS states (Example 5.11), for lightlike translated wedge algebras in the free massive field as in [CLR19], as well as in certain abelian (Example 5.12) and finite-dimensional (Example 5.1) situations. Nevertheless, it is a nonempty condition (Example 5.2). It may be seen as reminiscent of geometric modular action, as we shall see in Lemma 3.3 below.
If (L 0 , L 1 ) is in differential modular position, then we can define a projectorQ 0 on (a dense set of) X 1 by Because of item (ii) in the definition, this projector is actually real-orthogonal, and hence extends uniquely to a bounded operator on all of X 1 .
The spaces D ± 01 are somewhat difficult to explicitly describe in examples, we therefore give more directly applicable sufficient criteria for Def. 3.2. Then the pair (L 0 , L 1 ) is in differential modular position. In case (e), the associated projectorQ 0 is the identity.
Part (b) motivates the wording "differential modular", since it refers to the generator of the modular group only.
Proof. For (a), it suffices to show (by the assumed S 1 -graph density) that S 1 (f − , f + ) = 0 for all f + ∈ domR 1 ∩ D + 01 and all f − ∈ D − 01 . But for these, we can write since ı ⊕R 1 f + ∈ L 0 by assumption, and f − ∈ ker Q 0 = L ′ 0 . Items (b) and (d) are special cases of (a): If L 0 and L 1 are purely factorial, then for f For (c), we consider the case x ≥ 0, the other case being analogous; that is, U 1 is a strongly continous semigroup on img Q 0 = (L 0 ) f with respect to the K-norm, and on D + 01 with respect to the S 1 -graph norm. Now for f + ∈ D + 01 and ǫ > 0, consider Lemma 2.14). But also f + ǫ ∈ dom K 1 [EN00, Ch. II Lemma 1.3] and i ⊕ K 1 f + ǫ ∈ L 0 . Since vectors of the form (3.5) are a core for the generator on D + 01 , we can apply part (b). For (e), we use monotonicity of the entropy (Lemma 3.1) to show for hence by the Cauchy-Schwarz inequality for S 1 , we have S 1 (f − , f + ) = 0 for all f ± ∈ D ± 01 . Thus (L 0 , L 1 ) is in differential modular position, but also 1 −Q 0 = 0, i.e.,Q 0 = 1.

Families of subspaces
Closer to the applications we have in mind, we now proceed to a family of subspaces, labelled by a real parameter t; in particular, we are interested in the situation where the subspaces increase with the parameter.
Definition 3.4. A family of differential modular inclusions is a family (L t ) t∈R of closed subspaces of K which is increasing 5 (i.e., L s ⊂ L t for each s ≤ t) and where each pair (L s , L t ) (s, t ∈ R) is in differential modular position (Definition 3.2).
We will show later (Sec. 4) that the usual notion of (single-particle) half-sided modular inclusions [Bor00,Lon07] is a special case of Def. 3.4. However, the notion of differential modular inclusions is more general: It also applies to other situations where the modular group acts geometrically (Example 5.11) or where the space L t takes discrete steps (Example 5.1). Also, notice that Def. 3.4 is invariant under monotonous reparametrizations of the parameter t, whereas half-sided modular inclusions are not.
We note that for t ≤t, Lemma 3.1 gives us a canonical map ρ tt : Xt → X t which fulfills ϕ t = ρ tt • ϕt, and ρ tt ≤ 1. With respect to this inclusion map, we can now formulate some compatibility properties for the projectorsQ s on X t .
Lemma 3.5. If (L t ) t∈R is a family of differential modular inclusions, then: (a) For s ≤ŝ and any t, the projectorsQ s andQŝ on X t fulfilQ s ≤Qŝ.
(b) For any s and t ≤t, letQ s be the extension of Q s to X t andQ s the corresponding extension to Xt. We haveQ s • ρ tt = ρ tt •Q s .
(Because of the last property, we will not indicate the dependence ofQ s on the extension space X t beyond the proof of this lemma.) Proof. For (a), note first that ker Q s = L ′ s and similarly forŝ. Since L s ⊂ Lŝ, this yields (3.7) Now for any f = f + + f − ∈ Dŝ t , compute By density of ϕ t Dŝ t in X t , we obtain (using orthogonality of the projectors), (3.10) By density of ϕtD st in Xt, we concludeQ s • ρ tt = ρ tt •Q s .

Derivatives of the entropy
For a family of differential modular inclusions, we now investigate how the entropy S t (f, f ) of a given vector f depends on the parameter t; here we take f ∈D := ∩ t∈R dom S t . Actually, in order to study the "bulk" vs. "boundary" terms mentioned in the introduction, we consider the function T f : R 2 → R given by we have T f (t, t) = S t (f ), and we aim at estimates for d 2 S t /dt 2 in terms of the partial derivatives of T f , which will in general exist only in the sense of distributions. Crucial to this analysis are certain monotonicity properties of T f , in particular on the cones C ± := {(s, t) ∈ R 2 : ±(s − t) ≥ 0}. (c) Along the diagonal, it is increasing, i.e., T f (t, t) is increasing in t.
Item (c) above implies dS t (f )/dt ≥ 0, at least in the sense of distributions. For d 2 S t (f )/dt 2 , we will derive estimates stemming from item (d). For simplicity, let us first assume that T f is smooth outside the diagonal s = t, and at least C 1 at the diagonal. Proposition 3.7. Let f ∈D. Suppose that T f is of class C 1 , and that there are functionsT Proof. Since T f is C 1 , Lemma 3.6(b) implies ∂T f /∂s| s=t = 0, and we can differentiate this relation along the diagonal to yield ∂ 2T ± ∂s 2 s=t + ∂ 2T ± ∂s∂t s=t = 0. (3.16) On the other hand, S t =T ± (t, t), which yields together with (3.16), (3.17) Now ∂ 2 T f /∂s∂t vanishes on C + by Lemma 3.6(b), and is nonnegative on C − by Lemma 3.6(d); hence the result follows.
In other words, d 2 S f /dt 2 is bounded above und below by a "bulk term" (determined by the change of modular data in R t ), but the lower bound may allow for a positive "boundary term" (involving also a change inQ s ).
It is instructive to look at estimate (3.15) in specific examples. In certain situations, in particular in the conformal U (1)-current in the vacuum (Example 5.3), one has ∂ 2 T f /∂t 2 = 0 on C − , and the only contribution to d 2 S/dt 2 is the "boundary term" ∂ 2 T f /∂s∂t ≥ 0. Thus (3.15) implies convexity of the entropy in t in this case. However, in other situation, such as thermal states on the conformal U (1)-current (Example 5.11), or even when just reparametrizing a half-sided modular inclusion (Example 5.4), the "bulk term" ∂ 2 T f /∂t 2 need not vanish, and indeed can take any sign. Thus S t (f ) need not be convex in t, while the estimate (3.15) still holds.
We now want to establish a generalization of Prop. 3.7 without smoothness assumptions on T f . In preparation, we first prove: Lemma 3.8. For almost every t ∈ R, the function T f is continuous at the point (t, t).
Proof. The map t → T f (t, t) is monotonic, hence continuous almost everywhere; we fix a point t of continuity. Consider a sequence (s n , t n ) which converges to (t, t), and set u n := min{s n , t n }, v n := max{s n , t n }. Since T f is increasing in both variables by Lemma 3.6(a),(b), we have (3.18) As n → ∞, both sides of this inequality tend to T f (t, t), showing that T f is continuous (in two variables) at (t, t).
Further, we note that S t and T f are locally integrable (due to their monotonicity properties) and hence can be understood as distributions in C ∞ c (R) ′ and C ∞ c (R 2 ) ′ respectively. Regarding test functions, we fixfor all what follows-a nonnegative function h ∈ C ∞ c (R + ) with h = 1, and for any g ∈ C ∞ c (R) and ǫ > 0, which has support in the interior of C ± . The dual pairing between distributions and test functions will be denoted as · , · . With this notation, our generalisation of Prop. 3.7 to the non-smooth case is: Theorem 3.9. Let f ∈D. For any nonnegative g ∈ C ∞ c (R), one has (3.20) Proof. Due to local boundedness of T f , we have by dominated convergence together with Lemma 3.8. After a change of coordinates (s = t + u), this equality reads (3.22) Now by Lemma 3.6, the partial derivatives by s vanish in the interior of C + , and ∂T f /∂s∂t ≥ 0 in the interior of C − , yielding the proposed result.
Note the extra boundary term ∂ 2 T f /∂s 2 on the left-hand side of (3.20), which may have any sign. This term indeed occurs in Examples 5.1 and 5.13 and saturates the inequality there, hence cannot be omitted.
Thus convexity (d 2 S/dt 2 ≥ 0) can fail or a number of reasons. This is already apparent from our definitions: our notion of a "family of differential modular inclusions" in Definition 3.4 is invariant under monotonous reparametrizations of the parameter t, while convexity of S t is clearly not preserved under such reparametrizations in general. In fact, under mild conditions (e.g., if S t is strictly monotonous and at least continuous, but without restrictions on the second derivative), there exists a monotonous reparametrization of the family such that the resulting entropy function is convex (in fact, linear).

Half-sided modular inclusions
In this section, we show that the usual notion of half-sided modular inclusions of algebras [Bor00], via its analogue on the level of symplectic Hilbert spaces [Lon07], fits into the framework of this paper; more specifically, every half-sided modular inclusion yields a family of differential modular inclusions in the sense of Def. 3.4.
To that end, we first analyze an explicit example of half-sided modular inclusions (in a sense, the smallest nontrivial one), namely, the symplectic spaces of the conformal U (1)-current in the vacuum state (Sec. 4.1). For this model, convexity of the entropy was shown to hold in [Lon20]; we show that it fits within our framework of family of differential modular inclusions. Then, we decompose a general half-sided modular inclusion of symplectic Hilbert spaces into direct summands equivalent to the U (1)-current or to a trivial inclusion, thus lifting our results to the general case.
However, let us first note that our structures are indeed preserved under taking direct sums.
(b) If L n ⊂ K n are closed subspaces, and L := ⊕ n∈I L n , then we have for f = n∈I f n ∈ K, (4.1) (c) Suppose that, for each n ∈ I, {L n t } t∈R , with L n t ⊂ K n , is a family of differential modular inclusions for (K n , τ n , σ n ). Then {L t } t∈R := {⊕ n∈I L n t } t∈R is a family of differential modular inclusions for (K, τ, σ); and for f = n∈I f n ∈ ∩ t dom S Lt , we have where T n fn is the function (3.11) associated with the family {L n t }.
Proof. where D st is the subspace defined in (3.2) relative to the pair of subspaces (L t , L s ) in K. Since the family of subspaces {L n t } t∈R is by hypothesis a differential modular inclusion, we can find for every f ∈ dom(S Lt ) a sequence {g k } k∈Z+ ⊂D st , defined as (g k ) n := 0 if n > k, and such that for n ≤ k. We thus have by (4.1) which converges to 0 as k → ∞ since f has finite entropy.-Finally, one verifies that also the projectorsQ t and dom S Lt decompose along the direct sum, hence Eq. (4.2) follows from (4.1).

The U(1)-current in the vacuum
We consider the symplectic space for the U (1)-current, namely (in "configuration space" representation) C ∞ c (R) equipped with the symplectic form for f, g ∈ C ∞ c (R). The vacuum state is the pure quasifree state induced by the bilinear form wheref denotes the Fourier transformf The closure of C ∞ c (R) in the topology induced by τ is K = L 2 C (R + , p dp). This is a complex Hilbert space with complex scalar product ·, · and indeed, Thus, (K, τ, σ) is a pure symplectic Hilbert space (see Remark 2.3). Let I be the set of open, proper (bounded or unbounded) intervals of R. For an interval I ∈ I, let L U(1) (I) be the closure of C ∞ c (I) in K. The net {L U(1) (I)} I∈I is a local net of standard and factorial 6 subspaces of K, the well known U (1)-current net at single-particle level (restricted to the real line R). Its extension to the circle S 1 is covariant with respect to the action of the lowest weight 1 positive energy irreducible representation of the Möbius group, V . The latter, restricted to the subgroup P generated by translations and dilations (denoted by t → ϑ(t) and s → δ(s) respectively), is given explicitly on K = L 2 (R + , p dp) by This yields the unique irreducible, strictly positive energy representation of the group P; see, e.g., [Fol94, Section 6.7]. For brevity, for t ∈ R, we denote by L U(1) t := L U(1) ((−∞, t)), ∆ t := ∆ L U (1) t , K t := − log(∆ t ) and with mild abuse of notation we omit the identification between the configuration space representation and L 2 C (R + , p dp). By the Bisognano-Wichmann theorem for Möbius covariant local nets of standard subspaces [Lon07, Theorem 3.3.1] we have that ∆ −is 0 = V (δ(−2πs)), (4.10) and ∆ t for other t is then determined by translation covariance; in particular we get ("in configuration space") (4.11) Let Q t denote the projection (2.16) relative to the subspace L U(1) t ; since the space is factorial, it acts by (4.12) for almost all x ∈ R, where Θ denotes the Heaviside function.
One then immediately finds for the relative entropy by applying formula (2.25): Further, the spaces fit into our framework of differential modular inclusions (Definition 3.4): } t∈R is a family of differential modular inclusions.
Proof. We must prove that, for every s, t ∈ R, conditions (i) and (ii) in Definition 3.2 hold for the pair of subspaces (L ). In fact, once (i) is shown, (ii) is obtained immediately from points (c) and (e) of Lemma 3.3, which apply since the modular group acts geometrically by Eq. (4.10). Now for condition (i) in Definition 3.2, note that C ∞ c ((−∞, t)) ⊂ L U(1) t is a core for the generator , as it is a dense invariant subset of dom ı ⊕ K t ↾ L U(1) t [EN00, Proposition 1.7, Chapter 2]. Using Lemmas 2.15 and 2.16, we find that Thus to conclude the proof we only have to show that vectors in can be approximated by vectors in L where D st is defined in (3.2). Suppose s ≤ t; the proof for s > t is very similar.
Note thatD (4.14) which, by (4.13), is an isometry if C ∞ c ((−∞, t)) is equipped with the norm · t . To get the claim we show that the closure of ϕ(D st ) is the whole space To that end, we check that the orthogonal complement of ϕ( for all f ∈D st implies that g(x) = c t−x for Lebesgue-almost all −∞ < x < s with some constant c. But such g is not in L 2 ((−∞, s), (t − x)dx) unless c = 0. Thus g must vanish almost everywhere in (−∞, s), and by a similar argument, also in (s, t).
As a byproduct of the proof above, we see that the space X t can be identifed with L 2 ((−∞, t), (t − x)dx) via the map (4.15), with the projectorsQ s being multiplication with the characteristic function of (−∞, s).

Decomposition
In this section we show that the family of standard subspaces induced by a half-sided modular inclusion yields a family of differential modular inclusions (Definition 3.4). We start by recalling the notion of (singleparticle) half-sided modular inclusion and some of its relevant consequences following [Lon07].
Definition 4.5. Let K ⊂ H be real standard subspaces of a complex Hilbert space H. If the inclusion K ⊂ H is called a ±half-sided modular inclusion of standard subspaces.
In our context, we will work with −half-sided modular inclusions only. As above, let P denote the group generated by translations and dilations on the real line R, which we denote respectively with ϑ and δ, i.e. ϑ(t)(x) = x + t, δ(s)(x) = e s x for t, s, x ∈ R. We denote by δ 1 the one-parameter subgroup of P of dilations of the interval (1, ∞), i.e. δ 1 (s) = ϑ(−1)δ(s)ϑ(1).
A unitary representation V of the group P is said to have positive energy if the generator of the subgroup of translations, t → V (ϑ(t)), is a positive operator. It is said to be nonsingular if the kernel of the generator of translations is trivial.
Definition 4.7. Let K ⊂ H be a −half-sided modular inclusion and V be its induced representation of P from Theorem 4.6. K ⊂ H is said to be The following statement is the content of [Lon07, Corollary 4.3.2] which is obtained by decomposing the representation V into irreducibles. From the latter decomposition, we easily derive our desired result.
Proposition 4.9. Let K ⊂ H be a −half-sided modular inclusion of standard subspaces in a Hilbert space H. Then {V (ϑ(t))H} t∈R is a family of differential modular inclusions.
Proof. Combining Propositions 4.8 and 4.4 we have that {V (ϑ(t))H} t∈R decomposes into a direct sum of families of differential modular inclusions, thus the conclusion follows by Lemma 4.1.
Of course a similar statement can be obtained starting from a +half-sided modular inclusion.

Quantum mechanics
As the simplest, but instructive example, let us consider a finite-dimensional symplectic Hilbert space; for concreteness, K = C n with σ(f, g) = Im(f, g), where (f, g) denotes the standard scalar product on C n , and τ (f, g) = Re(f, M g) with some matrix M ≥ 1. (If M has no eigenvalue of 1, this may be interpreted as a thermal state on n independent harmonic oscillators, cf. [NT93], and M = 1 corresponds to the ground state of the oscillators.) Proof. For the first statement, by choosing a basis in which both M and E are diagonal and applying Lemma 4.1, it is sufficient to prove the statement for n = 1. In this case, either E = 0 (in which case the statement is trivial) or E = 1 (assumed in the following). Hence L = K and M = m1 with some m ≥ 1. Assume first m = 1. In that case, (K, τ, σ) is pure, and as in Remark 2.4, one has L ∞ = K ⊕ 0, L 0 = 0 ⊕ K. From Proposition 2.11, one sees that both sides of (5.1) are infinite (unless f = 0, in which case both are 0). Now let m > 1. In that case, one has D = −im −1 and One then computes the modular operator ∆ L of the spaces L = K ⊕ 0 and ı ⊕ L to be so that log ∆ L has the eigenvalues ±2 arcoth(m), and the projector Q L is obtained (for example by Lemma 2.6) as From Proposition 2.10, one then obtains (5.1).
For the differential modular inclusion, again by Lemma 4.1 it suffices to consider only the case n = 1. If E t = 0, then S t = 0 and (L s , L t ) is trivially in differential modular position; both sides of (5.2) vanish. If instead E t = E s = 1, i.e., L s = L t , differential modular position is clear and T f (s, t) = S t (f ) in agreement wih (5.2). Hence let E t = 1 and E s = 0. If m = 1, then f ∈ dom S t = {0} must vanish, and (5.2) holds trivially. If m > 1, then Q s = 0, D + st = {0}, D − st = K, one hasQ s = 0, and both sides of (5.2) vanish.
Of course, the same results for the entropy are obtained in the usual formalism representing thermal states of the harmonic oscillator as density matrices. It is interesting to note how our inequalities for d 2 S t /dt 2 work out in this example. Writing M = j m j E j in spectral decomposition, the terms in Theorem 3.9 are (in suggestive notation) so that the inequality (3.20) turns into an equality; note that the distribution δ ′ does not have a definite sign, hence finding nontrivial lower estimates would not be possible.
In the above example, our condition of differential modular position was satisfied because M leaves each subspace L t invariant. Clearly, this will not be true for more general subspaces. We provide an explicit counterexample: Example 5.2. In the above setting, let n = 2, M = diag(2, 3), let L 0 ⊂ K be the subspace spanned over R by the vectors (1, 1) and (i, 0), and let L 1 = K. Then (L 0 , L 1 ) is not in differential modular position.
Proof. By explicit matrix computation, one can find the modular operators related to L 0 and L 1 , and hence an explicit formula for Q 0 and S 1 . For f ∈ K, consider one finds that if f = (a, b) with a, b ∈ R, then δ = (b 2 − a 2 ) log 2.
(5.8) This is in general not positive, hence Q 0 cannot be orthogonal with respect to S 1 .
In the same situation, one finds that ; hence T f (s, t) defined as in (3.11) may be decreasing in s, and the conclusion of Lemma 3.6 fails.

Conformal U(1)-current, vacuum state
As an example from quantum field theory, we can take the conformal U (1)-current in the vacuum state, as already treated in Sec. 4.1. We briefly summarize the results here, and comment how the estimates on derivatives of the entropy work out in this case.
Example 5.3. Let (K, τ, σ) be the pure symplectic Hilbert space defined in Sec. 4.1 and let L t = L U(1) t ⊂ K. Then (L t ) t∈R is a family of differential modular inclusions, the space X t is isomorphic to We note here that T f is C 1 , as well as the restriction of smooth functions to the cones C ± ; one has so that the second derivative of S t is positive and given by a boundary term only. By the results of Sec. 4, a similar behaviour is exhibited by general half-sided modular inclusions. Namely, in the notation of Section 4.2, let K ⊂ H be a −half-sided modular inclusion in the complex Hilbert space H, K t := V (ϑ(t))H and f ∈ H. By using Lemma 4.1, we have that S t (f, f ) and T f (s, t) decompose along the direct sum provided by Proposition 4.8. Precisely, if f = n>0 f n + f 0 is the corresponding decomposition of f , with f 0 being the component relative to the trivial modular inclusion, where S t (f n , f n ) and T fn (s, t) with n > 0 are given by (5.9). The behaviour of the derivatives of S t (f, f ), at least when taking the f n to have suitably fast decay, is analogous to (5.10), noticing also that S t (f 0 , f 0 ), i.e., the contribution to the relative entropy given by the trivial half-sided inclusion component, is constant in t. As a particular example, this applies to the subspaces associated with lightlike shifted wedges in the real scalar free field, as in [CLR19].
The above situation is compatible with Proposition 3.7; however, the vanishing of ∂ 2 ∂t 2 T f is clearly a special feature of this particular family of subspaces. Even a reparametrization will remove it: Example 5.4. In Example 5.3, consider instead L t = L U(1) h(t) where h is a smooth, strictly increasing function. Then (L t ) t∈R is still a family of differential modular inclusions, but (5.11) Of course, this is still compatible with Proposition 3.7, but while the first term (the "boundary term") is still positive, the second derivative of S t will not be positive in general.

Conformal U(1)-current, thermal states
Let us now consider thermal (KMS) states on the conformal U (1)-current, as described in [BY99]. This examples illustrates, in particular, that different scalar products τ can be chosen with respect to the same symplectic form σ, and that this leads to different relative entropies.
Specifically, fixing β > 0, we choose on the non-completed space C ∞ c (R) the bilinear form 1 − e −βp p dp. (5.12) The associated quasifree state fulfills the KMS condition with respect to translations [BY99]. The completion of the symplectic space C ∞ c (R) with respect to τ β is K β := L 2 C (R + , p 1−exp(−βp) dp) as a real vector space; as before, we do not always denote the Forier transform explicitly. We apply the purification procedure described in Section 2.1: it is easy to see that where D is the multiplication operator by i (1 − e −βp ) on K β . In the polar decomposition D = C|D|, the operators |D| and C act by multiplication with (1 − e −βp ) and i, respectively. This induces a complex structure ı ⊕ on K ⊕ β := K β ⊕ K β by (2.3); let us denote the complex scalar product as ·, · β . For t ∈ R, we define L β t := C ∞ c ((−∞, t))) ⊂ K β where the bar indicates norm closure in K β . The bilinear form τ β is translation invariant, thus we have the following immediate proposition.
Example 5.11. In the symplectic Hilbert space (K β , τ β , σ) of the conformal U (1)-current with KMS state induced by τ β , consider L β t = C ∞ c (−∞, t). Then {L β t } t∈R is a family of differential modular inclusions, and for f ∈ C ∞ c (R), Computing the second derivative of the relative entropy, we have (5.28) Thus in the present case, the estimate in Proposition 3.7 bounds the second derivative of the entropy from below by its negative bulk term, i.e., the second term in (5.28).

Commutative algebras
It is instructive to consider also the case of abelian CCR algebras, i.e., subspaces L with L ⊂ L ′ .
Example 5.12. Let (X, M, µ) be a measure space such that K : For any two such subsets Y, Z, the pair (L Z , L Y ) is in differential modular position, andQ Z acts on X Y by multiplication with the characteristic function of Y ∩ Z.
Proof. By Remark 2.5, we have L ⊕ 0 = L 2 C (Y c , dµ), L a = L Y , L f = L ∞ = 0. The formula (5.29), and with it the proposed form of ϕ Y , then follows directly from Proposition 2.9; note that S Y is bounded and defined on all of K ⊕ . Also, noting that the projector Q Z (which acts by Q Z f = χ Z Im f ) is already orthogonal, we have D + ZY = iL 2 R (Z ∩ Y ), D − ZY = {f ∈ K : Im f ↾ Z = 0}, and one sees thatQ Z multiplies with χ Z∩Y in X Y .
As a special case, let us consider: Example 5.13. Let K = L 2 R (R), K ⊕ = L 2 C (R) with subspaces L t = L 2 R (−∞, t). Then L t is a family of differential modular inclusions, and we have S t (f, f ) = 2 t −∞ (Im f (x)) 2 dx and T f (s, t) = 2 min(s,t) −∞ (Im f (x)) 2 dx.
We note that in this example, the function T f is not C 1 . Clearly (Im f (t)) 2 , (5.30) thus S t will not be convex in general. Note that ∂ 2 T f /∂ 2 s = 2 d ds (Im f (s)) 2 and ∂ 2 T f /∂t 2 = 0 for s < t, so that the estimate in Theorem 3.9 is saturated.

Conclusions
In this paper, we have analyzed the relative entropy between coherent excitations of a general quasifree state on a CCR algebra, with respect to the algebra generated by a generic closed subspace. We gave an explicit description of the relative entropy in terms of single-particle modular data.
Also, we analyzed the change of the relative entropy along an increasing one-parameter family of subspaces, establishing an abstract notion of bulk and boundary changes. Convexity of the entropy (or the QNEC) is in general replaced by certain lower estimates of the second derivative, where both bulk and boundary terms can contribute.
An instrumental part of this analysis was the notion of differential modular position of two subspaces, meaning that the projector onto one subspace is orthogonal with respect to the scalar product induced by the entropy form of the other. While this is a nontrivial condition, we showed that it is fulfilled in a number of relevant examples; in particular it includes, but generalizes, the well-known notion of half-sided modular inclusions.
As the condition of differential modular position seems a fruitful tool, it would certainly be of interest to investigate whether it holds, possibly in a generalization, in a wider context than discussed here, both in other models of (linear) quantum fields and with respect to more general positions of subalgebras than treated in examples here. In particular, one would expect that it can be formulated employing notions of category theory, akin to the "locally covariant" setting of quantum field theory [BFV03]. We hope to report on this issue elsewhere.
Also, it would be of interest to generalize our framework beyond CCR algebras to general inclusions of von Neumann algebras; in the context of quantum field theory, this would correspond to models beyond linear fields. Clearly, a challenge is the limited availability of concrete examples beyond CCR algebras, in particular with sufficiently explicit descriptions of the relative modular operator. Possibly integrable models in low space-time dimensions, which are (fully or partially) known to fulfill quantum inequalities [BCF13,BC16], can provide some test cases in this respect.
A Relative entropy on C * and von Neumann algebras The notion of relative entropy for states on general von Neumann algebras was first introduced by Araki [Ara76, Ara77]. We recall its definition and relevant properties, following [OP04].
Let M be a von Neumann algebra on a Hilbert space H, let ω = ξ, · ξ a vector state (with some ξ ∈ H), and ϕ another state on M. The relative entropy between ω and ϕ (with respect to M) is defined as Here ω ′ ξ is the state ξ, · ξ restricted to M ′ , and ∆(ϕ/ω ′ ξ ) denotes the spatial derivative. In the case where both ω and ϕ are given by cyclic and separating vectors ξ, ψ, the relative modular ∆ ψ,ξ is defined and we have (see [ where the right-hand-side denotes the relative entropy with respect to the universal enveloping von Neumann algebra A * * of A andω,φ are the normal extensions of ω, ϕ to A * * . Suppose there is a representation π of A, π : A → B(H), where ω is a vector state, i.e., there is ξ ∈ H withω (π(a)) := ξ, π(a)ξ = ω(a), a ∈ A, and for which there is a normal stateφ on π(A) ′′ such that ϕ(a) =φ(π(a)), a ∈ A.
Then by applying Kosaki's formula for the relative entropy [OP04, Theorem 5.11], we have We recall the following properties of the relative entropy: