Abstract
The existence of a real linear space structure on the set of observables of a quantum system—i.e., the requirement that the linear combination of two generally noncommuting observables A, B is an observable as well—is a fundamental postulate of the quantum theory yet before introducing any structure of algebra. However, it is by no means clear how to choose the measuring instrument of a general observable of the form \(aA+bB\) (\(a,b\in {{\mathbb {R}}}\)) if such measuring instruments are given for the addends observables A and B when they are incompatible observables. A mathematical version of this dilemma is how to construct the spectral measure of \(f(aA+bB)\) out of the spectral measures of A and B. We present such a construction with a formula which is valid for general unbounded selfadjoint operators A and B, whose spectral measures may not commute, and a wide class of functions \(f: {{\mathbb {R}}}\rightarrow {{\mathbb {C}}}\). In the bounded case, we prove that the Jordan product of A and B (and suitably symmetrized polynomials of A and B) can be constructed with the same procedure out of the spectral measures of A and B. The formula turns out to have an interesting operational interpretation and, in particular cases, a nice interplay with the theory of Feynman path integration and the Feynman–Kac formula.
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1 Introduction
The elementary formulation of Quantum Theory in a complex separable Hilbert space \({{\mathsf {H}}}\) can be described as a nonBoolean probability theory. There, quantum states \(\mu \) are probability measures over the orthomodular separable \(\sigma \)complete lattice \({\mathscr {L}}({{\mathsf {H}}})\) of orthogonal projectors (the order relation being the standard inclusion of projection subspaces) which generalizes the notion of \(\sigma \)algebra (see, e.g., [4, 18, 22, 25, 27, 42]). The Hilbert space \({{\mathsf {H}}}\) depends on the physical system S one intends to study and the elements of \({\mathscr {L}}({{\mathsf {H}}})\) physically represent elementary propositions of S, also known as YES–NO elementary observables or tests about S. They are therefore assumed to have a definite operational meaning in terms of experimental devices. Commutativity of \(P,Q \in {\mathscr {L}}({{\mathsf {H}}})\) has the physical meaning of simultaneous measurability of the elementary observables represented by P and Q. In that case, P and Q are said to be compatible.
The issue we want to address in this work concerns the set \({\mathcal{O}}_S\) of observables of S. An observable A is primarily a collection of elementary propositions \(P^{(A)}_E\) labeled by real Borel sets \(E\in {\mathscr {B}}({{\mathbb {R}}})\). The operator \(P^{(A)}_E\) admits an explicit operational interpretation in terms of the statement “the outcome of the measurement of the observable A belongs to E.” We stress that there must be one (or several) measuring instrument(s) associated to the class \(\{P^{(A)}_E\}_{E \in {\mathscr {B}}({\mathbb {R}})}\). Sound physical and logical arguments (see, e.g., [18, 25, 42]) require that the collection \(\{P^{(A)}_E\}_{E \in {\mathscr {B}}({\mathbb {R}})}\) defines a \(\sigma \)Boolean algebra homomorphism form \({\mathscr {B}}({{\mathbb {R}}})\) to \({\mathscr {L}}({{\mathsf {H}}})\). In terms more familiar to physicists, \(\{P^{(A)}_E\}_{E \in {\mathscr {B}}({\mathbb {R}})}\) is a projectorvalued measure (PVM) also known as spectral measure. Among them, compatible observables A, B are by definition those whose associated PVMs are made of pairwise compatible projectors, i.e., \(P_E^{(A)}P_F^{(B)}=P_F^{(B)}P_E^{(A)}\) for all \(E,F \in {\mathscr {B}}({{\mathbb {R}}})\).
At this juncture, the spectral machinery establishes that there is a onetoone correspondence between PVMs over \({{\mathsf {H}}}\) and (generally unbounded) selfadjoint operators \(A: D(A) \rightarrow {{\mathsf {H}}}\). As a matter of fact, the following holds
We conclude that \({\mathcal{O}}_S\) is made of some selfadjoint operators \(A: D(A) \rightarrow {{\mathsf {H}}}\) and the natural question emerges about how large \({\mathcal{O}}_S\) is in the whole set of selfadjoint operators over \({{\mathsf {H}}}\).
As a matter of fact, it is generally assumed as a further postulate that \({\mathcal{O}}_S^{(b)}:={\mathcal{O}}_S\cap {\mathfrak {B}}({\mathsf {H}})\) is a linear subspace^{Footnote 1} of the real linear space of bounded^{Footnote 2} selfadjoint operators of \({{\mathfrak {B}}}({{\mathsf {H}}})\). This structure is later enriched [12, 18, 25, 40]) by adding in particular the socalled (nonassociative) Jordan product, and assuming suitable (weak) topological features compatible with the spectral machinery. The final construction turns out to be a concrete Jordan Walgebra in \({{\mathfrak {B}}}({{\mathsf {H}}})\) or, more generally, a concrete von Neumann algebra in \({{\mathfrak {B}}}({{\mathsf {H}}})\) when complex combination of observables is permitted. These structures are actually difficult to physically justify a priori. If assumed, they, however, promote the theory to a very high level of effectiveness in physics a posteriori.
Already sticking to the linear structure of the set of bounded observables, we argue that a longstanding (see, e.g., [9, 39]) open issue pops out, with a twofold nature, both physical and mathematical. Suppose that \(A,B \in {\mathcal{O}}_S^{(b)}\) and that we know their respective measuring instruments. If we pick out \(a,b \in {{\mathbb {R}}}\), in spite of the postulate about the linear structure of \({\mathcal{O}}_S^{(b)}\), there is no general way to associate a measuring instrument to \(aA+bB\) out of those of A and B. This obstruction is valid unless the observables aA and bB are compatible^{Footnote 3}. In that case, the instruments corresponding to the joint PVM of \(P^{(aA)}\) and \(P^{(bB)}\) can be exploited.
The mathematical version of the issue raised above is that no general formula is known determining the operator \(f(aA+bB)\)—and every projector \(P^{(aA+bB)}_E\) in particular—as a function of \(P^{(A)}\) and \(P^{(B)}\) when these PVMs do not commute. This work addresses the outlined problem from the mathematical side. We will prove—c.f. (32) and Theorem 2.5—that for a suitable class of continuous functions \(f: {{\mathbb {R}}}\rightarrow {{\mathbb {R}}}\), the following formula holds true:
This way the selfadjoint operator \(f(aA+bB)\) can be computed out of the PVMs of the selfadjoint operators A and B . Equation (2) is valid for generally noncommuting \(P^{(A)}\) and \(P^{(B)}\), also in the case of unbounded selfadjoint operators A and B under the condition that \(aA+bB\) is essentially selfadjoint over \(D(A)\cap D(B)\). The class of functions f is sufficiently large to include all polynomials when A and B are bounded, in particular \(aA+bB\) itself.
As one of the various byproducts of the abovementioned result for the case of A and B bounded, we also find an identity connecting the Jordan product \(A\circ B := \frac{1}{2}(AB+BA)\) to the generally noncommuting PVMs \(P^{(A)}\) and \(P^{(B)}\)—cf. Theorem 3.6.
Comparison with existing literature The assumption of the existence of a real linear space structure over the set of observables is crucial also in much more abstract, and apparently more operational, formulations of the quantum theory from [22] to [40]. Therein, the primary object is an abstract Jordan Banach \(^*\)algebra (or directly a \(C^*\)algebra), out of which the Hilbert space formulation is recovered a posteriori through the GNS construction. Observables are defined in terms of their expectation values (here properly interpreted as states), and it is postulated that given a pair of observables A and B and a corresponding pairs of reals a, b, there is an observable denoted by \(aA+bB\) whose expectation values are the linear combination of the expectation values of A and B with coefficients a and b. Though this observable is proved to be unique (because the states are reasonably supposed to separate the observables), no ideas are supplied to solve the problem we pointed out: how we can measure \(aA+bB\) if we know how to measure A and B when they are incompatible.
From the mathematical side, our results are entangled with the construction of a functional calculus for noncommuting operators. Several rigorous results exist in the literature about this subject. However, to the best of our knowledge, almost all are concentrated on two physically wellmotivated approaches: the generalization of Feynman’s functional calculus for Tordered products of operators and extensions of Weyl calculus—see [13, 15, 16, 28] for exhaustive reviews on these approaches—with several original contributions from outstanding authors [3, 23, 26]. The mathematical technology, the types of functional spaces and the interactions with some other mathematical objects like the Feynman–Kac integral share some similarities with the content of in this work—c.f. Sect. 3.2. However, to authors’ knowledge, none of those papers presents an integral expansion like our formula (2) where (a) a joint integral with respect to the noncommuting spectral measures of the involved operators shows up and (b) the physically suggestive averaged value of spectral parameters takes place—c.f. Sect. 5.
Structure of the work The paper is organized as follows. After recalling some general facts and the general notation used throughout, in Sect. 2 we tackle the problem raised above first in the finitedimensional case and next in the infinitedimensional case. Dealing with a pair of selfadjoint operators A, B in a complex Hilbert space and a continuous bounded function \(f: {{\mathbb {R}}}\rightarrow {{\mathbb {C}}}\) of a certain class, our main result consists of a formula where the operator \(f(aA+bB)\) is written as the (strong) limit of a sequence of certain operatorvalued integrals whose measure is an alternating product of spectral measures of A and B. As a matter of fact, we prove Eq. (9) in the finitedimensional case and Eq. (32) in the much harder infinitedimensional case. Section 3 is devoted to study some applications: In particular, we present a (fairly explicit) construction for the PVM of \(aA+bB\) and the Jordan product \(A\circ B\) in terms of the PVM of A and B. Eventually, we discuss the nice interplay with both the theory of Feynman integration in the phase space and the socalled Feynman–Kac formula. Section 4 contains some counterexamples which demonstrate how part of the structure introduced in the infinitedimensional case cannot be improved. In Sect. 5, we discuss the physical interpretation of the constructed formalism in the finitedimensional case where no technical issues take place, allowing us to focus directly on physics. A short summary ends the paper.
General conventions and notation We adopt throughout the paper the standard definition of complex measure [35], as a map \(\mu :\Sigma \rightarrow {{\mathbb {C}}}\) which is unconditionally \(\sigma \)additive over the \(\sigma \)algebra \(\Sigma \). With this definition, the total variation \(\mu  :=\mu (\Sigma )\) turns out to be finite. By \({\mathscr {B}}(X)\), we denote the Borel \(\sigma \)algebra over a topological space X and \(L^p(X, \nu )\) denotes the standard \(L^p\) space with respect to a positive Borel measure \(\nu \) [35] (in case \(\nu \) is complex, the associated \(L^p\) spaces are those referred to \(\nu \)). By \(L^p({{\mathbb {R}}}, \hbox {d}x)\) (also with \(\hbox {d}y\) in place of \(\hbox {d}x\)), we mean the \(L^p\) space with respect to Lebesgue measure (viewed as a Borel measure) on \({{\mathbb {R}}}\). In case the measure \(\nu \) is defined on a generic \(\sigma \)algebra \(\Sigma \) over the set X, we use the more precise notation \(L^p(X, \Sigma , \nu )\). If \(E\subset X\), for any given set X, then the indicator function \(1_E\) of E is defined as \(1_E(x):= 1\) if \(x\in E\) and \(1_E(x)=0\) if \(x\in X {\setminus } E\).
A Hilbert space is always assumed to be complex. We assume the usual convention concerning standard domains of composition of operators over a Hilbert space \({{\mathsf {H}}}\), \(A:D(A) \rightarrow {{\mathsf {H}}}\) and \(B: D(B) \rightarrow {{\mathsf {H}}}\) with \(D(A), D(B) \subset {{\mathsf {H}}}\) linear subspaces: (i) \(D(BA) := \{\psi \in D(A) \,\, A\psi \in D(B)\}\); (ii) \(D(A+B):= D(A)\cap D(B)\); (iii) \(D(aA):=D(A)\) for \(a\in {{\mathbb {C}}}{\setminus } \{0\}\) and \(D(0A):= {{\mathsf {H}}}\). These requirements yield in particular \(D(aA+bB) = D(A)\cap D(B)\) if \(ab \ne 0\). We define \(A^k := A \cdots (k \text{ times})\cdots A\) if \(k=1,2,\ldots \) and \(A^0:=I\). By \(A\subset B\) we mean that \(D(A) \subset D(B)\) and \(B_{D(A)}=A\).
We denote by \(A^*:D(A^*) \rightarrow {{\mathsf {H}}}\) the adjoint operator of a densely defined operator \(A: D(A) \rightarrow {{\mathsf {H}}}\) and by \({\overline{A}}\) its closure. A densely defined operator A is selfadjoint if \(A^*=A\). The operator A is essentially selfadjoint if \(A\subset A^*\) and \({\overline{A}}\) is selfadjoint. We denote by \({{\mathfrak {B}}}({{\mathsf {H}}})\) the unital \(C^*\)algebra of bounded everywhere defined operators over the Hilbert space \({{\mathsf {H}}}\), and \({\mathscr {L}}({{\mathsf {H}}})\subset {{\mathfrak {B}}}({{\mathsf {H}}})\) denotes the lattice of orthogonal projectors: \(P=P^*=PP\).
The spectrum of an operator A is always denoted by \(\sigma (A)\). According to the spectral theory (details, e.g., in [25, 34]), if \(T: D(T) \rightarrow {{\mathsf {H}}}\) is a generally unbounded selfadjoint operator in \({{\mathsf {H}}}\) and \(g: {{\mathbb {R}}}\rightarrow {{\mathbb {C}}}\) is measurable, then one has
Above, \( \mu ^{(T)}_{\phi , \psi }(E) := \langle \phi P^{(T)}_E\psi \rangle \) if \(E\in {\mathscr {B}}({{\mathbb {R}}})\) defines a regular complex Borel measure, which is positive if \(\psi =\phi \), and \(\{P^{(T)}_E\}_{E\in {\mathscr {B}}({{\mathbb {R}}})}\) is the projectionvalued measure (PVM)—also known as a spectral measure—uniquely associated with T. The righthand side of (3) can be defined [36]^{Footnote 4} as the unique operator T on D(g(T)) such that
The support of \(P^{(T)}\) coincides with the spectrum \(\sigma (T)\), and the integration in (3) can be restricted accordingly without affecting the identity. The spectral decomposition of T is nothing but (3) with \(g : {{\mathbb {R}}}\ni \tau \mapsto \tau \in {{\mathbb {R}}}\) and the spectral theorem just states that this decomposition exists and \(P^{(T)}\) is uniquely determined by T.
2 From \({{\mathbb {C}}}^n\) to an infinitedimensional Hilbert space
2.1 The finitedimensional Hilbert space case
The finitedimensional case is a comfortable arena where building up our formalism, since no problems related to domains and choices of topologies take place. Let us therefore suppose that \({{\mathsf {H}}}\) is finite dimensional. Without loss of generality, we can assume \({{\mathsf {H}}}= {{\mathbb {C}}}^k\). From the elementary spectral theory [37], we define
for every function \(g: {{\mathbb {R}}}\rightarrow {{\mathbb {R}}}\) and every selfadjoint operator T, where T is a \(k\times k\) Hermitian matrix \(T: {{\mathsf {H}}}\rightarrow {{\mathsf {H}}}\). The spectrum \(\sigma (T)\subset {{\mathbb {R}}}\) of T denotes its set of eigenvalues and \(P^{(T)}_\tau \) indicates the orthogonal projector onto the eigenspace of \(\tau \in \sigma (T)\), so that \(\{P_\tau ^{(T)}\}_{\tau \in \sigma (T)}\) completely determines the PVM \(P^{(T)}\) of T. No technical snags pop out with the sum in (5), since \(\sigma (T)\) is a nonempty set of at most \(k= \dim ({{\mathsf {H}}}) <+\infty \) elements.
We now focus on a couple of selfadjoint operators \(A: {{\mathsf {H}}}\rightarrow {{\mathsf {H}}}\), \(B: {{\mathsf {H}}}\rightarrow {{\mathsf {H}}}\) with, in general, \(AB \ne BA\). We intend to write \(f(aA+bB)\) in terms of the PVMs \(P^{(A)}\) and \(P^{(B)}\) for \(a,b\in {{\mathbb {R}}}\) and where \(f: {{\mathbb {R}}}\rightarrow {{\mathbb {C}}}\) is a sufficiently regular function. For technical reasons which will be evident shortly, we henceforth assume that: (i) \(f : {{\mathbb {R}}}\rightarrow {{\mathbb {C}}}\) is continuous; (ii) f belongs to \(L^1({{\mathbb {R}}}, \hbox {d}x)\); (iii) the inverse Fourier transform \(\check{f}(t) := \frac{1}{2\pi }\int _{{\mathbb {R}}}f(x) \hbox {e}^{itx} \hbox {d}x\) belongs to \(L^1({{\mathbb {R}}}, \hbox {d}x)\). Every \(f\in {\mathscr {S}}({{\mathbb {R}}})\) in particular satisfies the said three hypotheses. Assuming (i),(ii) and (iii), the pointwise inversion theorem of the Fourier transform is valid: \(f(x) = \int _{{\mathbb {R}}}\check{f}(t) \hbox {e}^{itx} \hbox {d}t\) for every \(x\in {\mathbb {R}}\).
The pivotal tool underpinning our result is the celebrated Trotter formula,
whose convergence is here referred to every normed topology on \({{\mathfrak {B}}}({{\mathsf {H}}})\), since that (Banach) space is finite dimensional. Spectrally decomposing the exponentials on both sides into a finite linear combinations of matrices according to (5) and using of Lebesgue’s dominated convergence theorem term by term while integrating both sides against \(\check{f}(t)\), we have,
Exploiting (5), identity (7) can be expanded as
Since \(f(x) = \int _{{\mathbb {R}}}\check{f}(t) \hbox {e}^{itx} \hbox {d}t\) and taking (5) into account on the lefthand side, we obtain the prototype of our general formula
In \({{\mathsf {H}}}= {{\mathbb {C}}}^k\), it is not difficult to prove that \(ABBA=0\) implies \(\big (\hbox {e}^{i\frac{t}{N}aA} \hbox {e}^{i\frac{t}{N}aB}\big )^N = \hbox {e}^{it(aA+bB)}\,. \) Hence, following our derivation of (8), the limit on the righthand side of (8) is not necessary since its argument turns out to be constant in N. Therefore, for commuting A and B, equation (8) reduces to
which is nothing but the usual spectral decomposition of the lefthand side with respect to the joint PVM of A and B.
A physically important case of (9) would be obtained by choosing \(f= 1_{[\alpha ,\beta )}\) (the indicator function of the set \([\alpha ,\beta )\)). As a matter of fact, \(1_{[\alpha ,\beta )}(aA+bB) = P^{(aA+bB)}_{[\alpha ,\beta )}\) is the spectral projection of \([\alpha ,\beta )\) and this family of projectors, when \(\alpha < \beta \), includes the full information of the PVM of \(aA+bB\). Unfortunately, such f does not satisfy (i) and (iii); hence, a further regularization procedure is necessary by means of a family \(1^{(\epsilon )}_{[\alpha ,\beta )} \in {\mathscr {S}}({\mathbb {R}})\) suitably converging to \(1_{[\alpha ,\beta )}\) as \(\epsilon \rightarrow 0^+\). In this way, the identity
can be established. We shall prove it later in a much more general context as identity (38).
The requirement \(f, \check{f} \in L^2({{\mathbb {R}}},\hbox {d}x)\) can be relaxed making stronger the regularity requirement on f as a consequence of the following argument. If f, g satisfy (i), (ii), (ii) and also \(f(x)=g(x)\) for \(x \in [\Vert aA\Vert \Vert bB\Vert , \Vert aA\Vert + \Vert bB\Vert ]\), where the norm is the operator norm, then the wellknown general estimate for selfadjoint operators that \(\sigma (T) \subset [\Vert T\Vert ,\Vert T\Vert ]\), yields both
from (5), and
It is consequently safe to extend the validity of (8) to every complex valued \(f\in C^\infty ({{\mathbb {R}}})\) simply smoothly changing f to a function of \({\mathscr {S}}({{\mathbb {R}}})\) outside the interval \([\Vert aA\Vert \Vert bB\Vert , \Vert aA\Vert + \Vert bB\Vert ]\). In particular, f can be chosen as a polynomial of a single real variable. In this way, we also obtain the elementary Jordanalgebra operations on A and B written in terms of the PVMs of A and B as the second identity below. If \(a,b \in {{\mathbb {R}}}\),
and
The former is simply obtained from (8) choosing \(f(s)=s\). The latter arises from a more involved though elementary procedure. The lefthand side of (13) can be written as
where \(f(s):=s^2\), \(g(s)= s^2\), \(a=b=1\), \(a'=1\), \(b'=0\), \(a''=0\), \(b''=1\). Linearity in f of the righthand side of (8) (also with different constants a, b) immediately gives rise to (13). A more detailed discussion will appear in Sect. 3, where (13) is extended to polynomials (Theorem 3.6).
With an argument similar to the one leading to (11) and using the fact that \(\sigma (aA+bB)\) is a finite discrete set of reals, we achieve another useful result. If \(\beta \not \in \sigma (aA+bB)\), identity (10) can be alternatively written
where \(1'_{[\alpha ,\beta )} \in {\mathcal{D}}({{\mathbb {R}}})\) is a map which attains the constant value 1 over \([\alpha , \beta )\) and smoothly vanishes on \(\sigma (aA+bB) {\setminus } [\alpha ,\beta )\).
When trying to extend (8) to the case of a general (separable) Hilbert space \({{\mathsf {H}}}\) for generally unbounded selfadjoint operators A and B, several evident technical issues arise. First of all, usual domain problems have to be fixed. These problems are tantamount to corresponding domain issues with Trotter’s formula which are well known and definitely fixed [33, Theorem VIII.31]. A sufficiently general setup consists of assuming that \(aA+bB\) is essentially selfadjoint over its natural domain \(D(A)\cap D(B)\) (if \(ab\ne 0\)). A much harder problem is the interpretation of the operatorvalued integral appearing in the righthand side of (8), especially in case the spectrum of either A or B includes a continuous part. Actually, problems of a similar nature arise also when A and B have pure point spectra, but \({{\mathsf {H}}}\) is infinite dimensional. In the following sections, we will address those technical problems and other related ones, ending up with a wide generalization of (8)—c.f. Theorem 2.5.
2.2 The unital Banach algebra of complex Borel measures
Before entering the technical details of the core of the paper, it is necessary to introduce the space of functions we will use on both sides of the extension of (8).
Definition 2.1
The space of complex measures on \({{\mathbb {R}}}\) denoted by \({\mathscr {M}}({{\mathbb {R}}})\) is the complex linear space of \({\mathbb {C}}\)valued \(\sigma \)additive maps \(\nu : {\mathscr {B}}({{\mathbb {R}}}) \rightarrow {{\mathbb {C}}}\). The space of Fourier transforms of complex measures on \({{\mathbb {R}}}\) consists of the complex linear space \({\mathscr {F}}({\mathbb {R}})\) of functions of the form
for some \(\nu \in {\mathscr {M}}({{\mathbb {R}}})\). \(\square \)
The linear map
is injective (this is a straightforward extension of [5, Theorem 26.2]) so that it defines a linear isomorphism. From the standard properties of Fourier transform, it is not difficult to prove that \({\mathscr {F}}\) includes the maps satisfying (i), (ii), (iii) we used in Sect. 2.1. Furthermore,
Above, \(C_b({{\mathbb {R}}})\) is the commutative unital Banach algebra (with norm \(\Vert \cdot \Vert _\infty \)) of bounded continuous complexvalued functions over \({{\mathbb {R}}}\), \({\mathscr {S}}({{\mathbb {R}}})\) and \({\mathcal{D}}({{\mathbb {R}}})\) are, respectively, the space of Schwartz (complex) functions and the space of the (complex) test functions over \({{\mathbb {R}}}\), and \({\mathscr {S}}'({{\mathbb {R}}})\) and \({\mathcal{D}}'({{\mathbb {R}}})\) denote the associated spaces of distributions.
The linear space \({\mathscr {M}}({{\mathbb {R}}})\) turns out to be a commutative unital Banach algebra where (a) the product of two measures \(\nu \) and \(\nu '\) is their convolution \(\nu * \nu '\), (b) the unit is the Dirac point mass \(\delta _0\) concentrated at 0 and (c) the norm of a measure \(\nu \) is defined as its total variation \(\Vert \nu \Vert =\nu ({{\mathbb {R}}})\). \({\mathscr {M}}({{\mathbb {R}}})\) also admits a normpreserving unitpreserving antilinear involution given by the complex conjugation of measure \(\nu ^* := {\overline{\nu }}\). The linear isomorphism (16) induces a unital commutative Banach algebra structure over \({\mathscr {F}}({{\mathbb {R}}})\) when defining \(\Vert f_\nu \Vert _{\mathscr {F}}:=\Vert \nu \Vert \). More precisely, the map F promoted to an isomorphism of Banach algebras transforms the convolution of measures into the pointwise product of corresponding functions and the unit of \({\mathscr {M}}({{\mathbb {R}}})\) to the constant function 1. The involution of \({\mathscr {M}}({{\mathbb {R}}})\) becomes the normpreserving unitpreserving antilinear involution over \({\mathscr {F}}({\mathbb {R}})\), given by \(f^*(x) := \overline{f(x)}\), the bar denoting the complex conjugation. The definition of \(\Vert f\Vert _{\mathscr {F}}\) easily implies
If \(f \in {\mathscr {S}}({{\mathbb {R}}})\) (or \({\mathcal{D}}({{\mathbb {R}}})\)), then \(f= f_\nu \) where \(\hbox {d}\nu = (2\pi )^{1} \check{f} \hbox {d}x\) and \(\check{f}(y) = \int _{{\mathbb {R}}}\hbox {e}^{ixy} f(x) \hbox {d}y\) is the Fourier antitransform of f. In this case
2.3 Regularized products of noncommuting PVMs of selfadjoint operators
This section and the subsequent one are devoted to extend formula (8) to the case of an infinitedimensional, though separable, Hilbert space \({{\mathsf {H}}}\). We will suppose that the operators A and B are unbounded selfadjoint operators with domains D(A) and D(B), respectively, and that their linear combination \(aA+bB\), for suitable \(a,b \in {{\mathbb {R}}}\), is essentially selfadjoint on its standard domain according to Sect. 1.
In other words, we want to construct a functional calculus and the spectral measure of the selfadjoint operator given by the closure \(\overline{aA+bB}\) out of the PVMs \(P^{(A)}, P^{(B)}\) of A and B, respectively, proving the following suggestive formula if \(\psi \in {{\mathsf {H}}}\) and \(f \in {\mathscr {F}}({{\mathbb {R}}})\):
The operator \(f\left( \overline{aA+bB}\right) \) on the lefthand side is independently defined by (3) and its domain is the whole \({{\mathsf {H}}}\) according to (3) since f is bounded.
As a first step, we address the problem of the interpretation of the operators
after the symbol of limit on the righthand side of (19). In fact, we cannot generally interpret the integration appearing in (20) like the one in (9), i.e., as referred to the joint PVM of N copies of \(P^{(A)}\) and \(P^{(B)}\) (see, e.g., [25, 34]). This is because we are focusing on the generic situation where \(P^{(A)}\) and \(P^{(B)}\) do not commute. In the general case, operators (20) are defined out of a regularized natural quadratic form we are going to introduce with the following crucial technical result. We stress that we will not use the hypothesis of essential selfadjointness of \(aA+bB\) at this stage of the construction.
Lemma 2.2
Let A and B be a pair of selfadjoint operators over the separable Hilbert space \({{\mathsf {H}}}\) as in (3), and \(Q:=\{Q_n\}_{n\in {{\mathbb {N}}}}\) a sequence of orthogonal projectors over respective finitedimensional subspaces such that \(Q_n \rightarrow I\) strongly as \(n\rightarrow +\infty \).
If \(\phi , \psi \in {{\mathsf {H}}}\) and \(N\in {\mathbb {N}}\), then the following facts are valid.
 (a):

For every \(n\in {{\mathbb {N}}}\), there is a unique complex Borel measure \(\nu _{\phi ,\psi ,Q}^{(N,n)}\) over \({{\mathbb {R}}}^{2N}\) such that
$$\begin{aligned} \nu ^{(N,n)}_{\phi ,\psi ,Q}(\times _{\ell =1}^NI_\ell \times J_\ell ):= \langle \phi  P^{(A)}_{I_1}Q_{n}P^{(B)}_{J_1}\cdots P^{(A)}_{I_N}Q_{n}P^{(B)}_{J_N}\psi \rangle , \end{aligned}$$(21)with \(I_\ell , J_\ell \) arbitrary Borel sets in \({{\mathbb {R}}}\). The support of the measure satisfies
$$\begin{aligned} \text{ supp }(\nu ^{(N,n)}_{\phi ,\psi ,Q}) \subset \underbrace{\sigma (A)\times \sigma (B) \times \cdots \times \sigma (A) \times \sigma (B)}_{2N \ \mathrm { times}}\,. \end{aligned}$$(22)  (b):

For every \(f \in {\mathscr {F}}({{\mathbb {R}}})\) and, independently of the choice of the sequence \(\{Q_n\}_{n\in {{\mathbb {N}}}}\), the following limit holds for \(a,b \in {{\mathbb {R}}}\):
$$\begin{aligned}&\lim _{n\rightarrow \infty } \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N}\sum _{l=1}^{N}(a\lambda _l+b\mu _l)\right) \mathrm{d}\nu ^{(N,n)}_{\phi ,\psi ,Q}(\lambda _1,\mu _1,\dots ,\lambda _N,\mu _N)\nonumber \\&\quad =\int _{{\mathbb {R}}}\left\langle \phi \left (\hbox {e}^{i \frac{t}{N}aA}\hbox {e}^{i \frac{t}{N}bB})^N\psi \right. \right\rangle \mathrm{d}\nu _f(t)\,, \end{aligned}$$(23)
Proof
See “1” \(\square \)
Analogously to the use of (4) to define the righthand side in (3), the idea is now to define the operator in (20) in order that the associated quadratic form coincides with the limit of the regularized sequences as on the lefthand side of (23).
Theorem 2.3
Let A and B be a pair of selfadjoint operators over the separable Hilbert space \({{\mathsf {H}}}\) as in (3), \(f\in {\mathscr {F}}\), and \(N\in {\mathbb {N}}\). For \(a,b \in {{\mathbb {R}}}\), there is a unique operator, denoted by
such that
Above, for every \(n\in {{\mathbb {N}}}\), the complex Borel measure \(\nu ^{(N,n)}_{\phi ,\psi ,Q}\) is uniquely defined by
for a sequence of finitedimensional orthogonal projectors \(Q:=\{Q_n\}_{n\in {{\mathbb {N}}}}\) with \(Q_n \rightarrow I\) strongly as \(n\rightarrow +\infty \). The limit in (25) is, however, independent of the choice of \(\{Q_n\}_{n\in {{\mathbb {N}}}}\).
The following further facts are true.

(i)
The map
$$\begin{aligned} {\mathscr {F}}\ni f \mapsto \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N} \sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) \hbox {d}P^{(A)}_{\lambda _1}\hbox {d}P^{(B)}_{\mu _1}\cdots \hbox {d}P^{(A)}_{\lambda _N}\hbox {d}P^{(B)}_{\mu _N}\in {\mathfrak {B}}({\mathsf {H}}) \end{aligned}$$is linear.

(ii)
The following inequality holds
$$\begin{aligned} \left \left \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N}\sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) \hbox {d}P^{(A)}_{\lambda _1}\hbox {d}P^{(B)}_{\mu _1} \cdots \hbox {d}P^{(A)}_{\lambda _N}\hbox {d}P^{(B)}_{\mu _N} \right \right \le \Vert f\Vert _{\mathscr {F}}\,. \end{aligned}$$(26) 
(iii)
If \(\phi ,\psi \in {{\mathsf {H}}}\), the restricted maps
$$\begin{aligned}&{\mathscr {S}}({{\mathbb {R}}})\ni f \mapsto \left\langle \phi \left \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N}\sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) \hbox {d}P^{(A)}_{\lambda _1}\hbox {d}P^{(B)}_{\mu _1}\cdots \hbox {d}P^{(A)}_{\lambda _N}\hbox {d}P^{(B)}_{\mu _N}\psi \right. \right\rangle \end{aligned}$$(27)$$\begin{aligned}&{\mathscr {S}}({{\mathbb {R}}})\ni f \mapsto \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N}\sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) \hbox {d}P^{(A)}_{\lambda _1}\hbox {d}P^{(B)}_{\mu _1}\cdots \hbox {d}P^{(A)}_{\lambda _N}\hbox {d}P^{(B)}_{\mu _N} \end{aligned}$$(28)are, respectively, a Schwartz distribution and a \({\mathscr {B}}({{\mathsf {H}}})\)valued Schwartz distribution. The same facts hold if replacing \({\mathscr {S}}({{\mathbb {R}}})\) with \({\mathcal{D}}({{\mathbb {R}}})\) and \({\mathscr {S}}'({{\mathbb {R}}})\) with \({\mathcal{D}}'({{\mathbb {R}}})\).

(iv)
If \(A, B \in {{\mathfrak {B}}}({{\mathsf {H}}})\) and \(\text{ supp }(f) \cap [\Vert aA\Vert \Vert bB\Vert , \Vert aA\Vert + \Vert bB\Vert ] = \varnothing \), then
$$\begin{aligned} \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N}\sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) \hbox {d}P^{(A)}_{\lambda _1}\hbox {d}P^{(B)}_{\mu _1}\cdots \hbox {d}P^{(A)}_{\lambda _N}\hbox {d}P^{(B)}_{\mu _N}=0\,. \end{aligned}$$ 
(v)
If \({\overline{z}}\) denotes the complex conjugate of \(z\in {\mathbb {C}}\), then
$$\begin{aligned}&\left[ \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N}\sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) \hbox {d}P^{(A)}_{\lambda _1}\hbox {d}P^{(B)}_{\mu _1}\cdots \hbox {d}P^{(A)}_{\lambda _N}\hbox {d}P^{(B)}_{\mu _N}\right] ^*\nonumber \\&\quad =\int _{{{\mathbb {R}}}^{2N}} \overline{f\left( \frac{1}{N}\sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) } \hbox {d}P^{(B)}_{\mu _1}\hbox {d}P^{(A)}_{\lambda _1}\cdots \hbox {d}P^{(B)}_{\mu _N}\hbox {d}P^{(A)}_{\lambda _N}\,. \end{aligned}$$(29)
Proof
If \(\nu _f := F^{1}(f)\) according to (15)–(16), the map appearing on the righthand side of (23), that is,
is by construction linear in f and \(\psi \), antilinear in \(\phi \) and satisfies
As a consequence, identity (23) permits us to exploit Riesz’ lemma defining the wanted operator as required and independently from the regularizing sequence \(\{Q_n\}_{n\in {{\mathbb {N}}}}\). Indeed, for any \(\psi ,f\), the map \(\phi \mapsto I^{(N)}_{\phi ,\psi }(f)\) defines a bounded antilinear functional, hence Riesz representation theorem allows to write the following identity
for a suitable vector \( \xi _f\in {{\mathsf {H}}}\) such that
The linear dependence of \(I^{(N)}_{\phi ,\psi }(f)\) on \(\psi \) yields the linearity of the map \(\psi \mapsto \xi _\psi :=L(\psi )\) as well. Finally, inequality (31) allows to prove that the operator L is bounded and by definition it coincides with (24). Linearity of \(f \mapsto I^{(N)}_{\phi ,\psi }(f)\) and (30) prove (i) and (ii).
Regarding (iii), we observe that from the continuity properties of the Fourier transform, \({\mathscr {S}}({{\mathbb {R}}}) \ni f_n \rightarrow 0\) in the \({\mathscr {S}}\)topology (as \(n \rightarrow +\infty \)) implies that the sequence of antitransforms \(\check{f}_n\) vanishes in the same topology, so that, in particular, \(\Vert \check{f}_n\Vert _{L^1({{\mathbb {R}}}, \hbox {d}x)} \rightarrow 0\). Since \(\Vert f_n\Vert _{\mathscr {F}}= (2\pi )^{1} \Vert \check{f}_n\Vert _{L^1({{\mathbb {R}}}, \hbox {d}x)}\) from (18), we have that \(\Vert f_n\Vert _{\mathscr {F}}\rightarrow 0\). The linear maps (27) and (28) are therefore \({\mathscr {S}}\)continuous in view of inequality (26) so that they are Schwartz distributions by definition. Since Schwartz distributions are distributions over \({\mathcal{D}}({{\mathbb {R}}})\), the result is also valid when restricting our map to \({\mathcal{D}}({{\mathbb {R}}})\).
(iv) First observe that \(\sigma (A) \subset [\Vert A\Vert ,\Vert A\Vert ]\) and \(\sigma (B) \subset [\Vert B\Vert , \Vert B\Vert ]\). At this juncture, inclusion (22) and definition (25) imply that the integration over \({{\mathbb {R}}}^{2N}\) on the righthand side of (25) can actually be restricted to the set determined by imposing \(\lambda _j \in [\Vert A\Vert ,\Vert A\Vert ]\) and \(\mu _j\in [\Vert B\Vert ,B\Vert ]\) for \(j=1,\ldots , N\), without affecting the final result. If the support of f is disjoint from \( [\Vert aA\Vert \Vert bB\Vert , \Vert aA\Vert +\Vert bB\Vert ]\), then \(f\left( \frac{1}{N}\sum _{j=1}^N (a\lambda _j+b\mu _j)\right) \) vanishes when \(\lambda _j \in [\Vert A\Vert ,\Vert A\Vert ]\) and \(\mu _j\in [\Vert B\Vert ,\Vert B\Vert ]\) so that the integral in (25) vanishes as well for every n, producing 0 as limit for \(n\rightarrow +\infty \).
The proof of (v) follows at once from the definitions. \(\square \)
Remark 2.4
(1) If \({{\mathsf {H}}}\) is finite dimensional, all \(Q_n\) on the righthand side of (21) can be removed, simply choosing \(Q_n=I\), finding the formulas achieved in Sect. 2.1. For infinitedimensional \({{\mathsf {H}}}\), there are cases where no complex measure satisfying identity (21) exists if \(Q_n=I\) for all n—c.f. Sect. 4.1.
(2) The existence of sequences \(\{Q_n\}_{n\in {{\mathbb {N}}}}\) strongly approximating the identity operator with finitedimensional projection spaces is equivalent to separability of \({{\mathsf {H}}}\). Hence, separability hypothesis cannot be relaxed. \(\square \)
2.4 Main result
We have reached a position to establish our main theorem when, in addition to the already assumed hypotheses on A and B, we use the requirement that \(aA+bB\) is essentially selfadjoint.
Theorem 2.5
Let A, B be selfadjoint operators on a separable Hilbert space, \(a,b\in {{\mathbb {R}}}\) and let us assume that \(aA+bB\) is essentially selfadjoint on \(D(aA)\cap D(bB)\). Then, the following facts hold for \(f\in {\mathscr {F}}({{\mathbb {R}}})\).
 (a):

Denote the strong operator limit by \(s\lim \). Then,
$$\begin{aligned} f\left( \overline{aA+bB}\right) = \text{ s }\lim _{N\rightarrow +\infty } \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N}\sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) \hbox {d}P^{(A)}_{\lambda _1}\hbox {d}P^{(B)}_{\mu _1}\cdots \hbox {d}P^{(A)}_{\lambda _N}\hbox {d}P^{(B)}_{\mu _N}\,, \end{aligned}$$(32)and a similar identity is valid if, keeping the lefthand side, we swap \(\hbox {d}P^{(A)}_{\lambda _j}\) and \(\hbox {d}P^{(B)}_{\mu _j}\) for \(j=1,2,\ldots , N\) on the righthand side.
 (b):

If the PVMs \(P^{(aA)}\) and \(P^{(bB)}\) commute (this fact holds in particular if either \(a=0\) or \(b=0\)), then
$$\begin{aligned} f\left( \overline{aA+bB}\right) = \int _{{{\mathbb {R}}}^{2N}} f\left( \frac{1}{N}\sum ^N_{n=1} (a\lambda _{n} + b\mu _{n})\right) \hbox {d}P^{(A)}_{\lambda _1}\hbox {d}P^{(B)}_{\mu _1}\cdots \hbox {d}P^{(A)}_{\lambda _N}\hbox {d}P^{(B)}_{\mu _N}\,, \end{aligned}$$(33)for every \(N\in {\mathbb {N}}\).
 (c):

If the PVMs \(P^{(A)}\) and \(P^{(B)}\) commute, then
$$\begin{aligned} \nu ^{(1,n)}_{\phi ,\psi ,Q}(I\times J)= \langle \phi  P^{(A)}_{I}Q_{n}P^{(B)}_{J}\psi \rangle \rightarrow \langle \phi  P^{(A,B)}_{I\times J}\psi \rangle \quad \text{ as } n\rightarrow +\infty , \end{aligned}$$where \(P^{(A,B)} : {\mathscr {B}}({{\mathbb {R}}}^2) \rightarrow {\mathscr {L}}({{\mathsf {H}}})\) is the joint PVM of A and B and the righthand side of (33)—defined as in (25)—with \(N=1\) can be interpreted as an integration with respect to that joint PVM.
Proof
(a) From now on, \(\nu _f := F^{1}(f)\) according to (15)–(16). For \(N\in {{\mathbb {N}}}\), we define the operator
as the unique operator \(S\in {{\mathfrak {B}}}({{\mathsf {H}}})\) such that
The operator
is analogously defined.
The former operator is already known. Indeed, from (23) and (25), we find
We now turn our attention to the operator in (34). Let \(P^{(\overline{aA+bB})}\) be the spectral measure of the selfadjoint operator \(\overline{aA+bB}\) and set \(\mu _{\phi , \psi }(E) = \langle \phi P^{(\overline{aA+bB})}(E)\psi \rangle \), \(E \in {\mathscr {B}}({{\mathbb {R}}})\), the complex Borel measure associated with \(\phi \) and \(\psi \). By standard functional calculus, by writing \(f\in {\mathscr {F}}\) as in (15) and exploiting Fubini’s theorem (all measures are finite and the integrand is bounded), we obtain:
In other words,
Taking advantage of (35) and (36), the thesis of the theorem can be rephrased to
Representing the lefthand side as an inner product and expanding it, taking the previous definitions into account, we find that the squared norm above equals
Fubini’s theorem permits us to rewrite the above integral as
where \(\hbox {d}\overline{\nu _f}(t) \otimes \hbox {d}\nu _f(s)\) is the product measure. By the Trotter product formula [33, Theorem VIII.31], which is valid in our hypotheses on aA and bB, both entries of the scalar product vanish as \(N\rightarrow +\infty \). This fact implies that the integral itself vanishes as a consequence of Lebesgue’s dominated convergence theorem, since the product measure is finite and the integrand is uniformly bounded in (t, s) as the involved operators are unitary. In summary, (37) is valid and the proof of (a) ends since the last statement is an obvious consequence of \(\overline{aA+bB}=\overline{bB+aA}\).
(b) Exploiting the structure of the proof of (a), the thesis is valid if, for every \(t\in {{\mathbb {R}}}\),
Let us prove that this identity is in fact true. Since \(P^{(aA)}\) and \(P^{(bB)}\) commute, referring to their joint PVM P, we have
From the general properties of the integral of bounded functions with respect to a given PVM,
Taking the strong limit as \(N\rightarrow +\infty \), Trotter’s formula yields
so that, using again \(\left( \hbox {e}^{i \frac{t}{N}aA}\hbox {e}^{i \frac{t}{N}bB}\right) ^N = \hbox {e}^{i taA}\hbox {e}^{i tbB}\), we find
as wanted.
(c) is evident from (b), the requirement that \(Q_n \rightarrow I\) strongly, the definition of joint PVM, and its elementary properties. \(\square \)
3 Some applications
3.1 The PVM of \(\overline{aA+bB}\) from \(P^{(A)}\) and \(P^{(B)}\)
As an application of Theorem 2.5, we prove that knowledge of the PVMs \(P^{(A)},P^{(B)}\) of A and B suffices to determine the PVM of \(\overline{aA+bB}\) among all PVMs over \({\mathbb {R}}\). We take advantage of the wellknown result that^{Footnote 5}\(P^{(\overline{aA+bB})}\) is known once the projectors \(P^{(\overline{aA+bB})}_{[\alpha ,\beta )}\) are known for all \(\alpha ,\beta \in {{\mathbb {R}}}\) with \(\alpha < \beta \).
Theorem 3.1
If A and B are as in Theorem 2.5 and \(a,b \in {{\mathbb {R}}}\), the following identity holds for every \(\alpha ,\beta \in {{\mathbb {R}}}\) with \(\alpha < \beta \),
where the \(\epsilon \)parametrized class of \({\mathscr {S}}({\mathbb {R}})\) functions
pointwise converges to \(1_{[\alpha ,\beta )}\) for \(\epsilon \rightarrow 0^+\).
Proof
Observing that \(\Vert 1_{[\alpha , \beta )}^{(\epsilon )}\rightarrow 1_{[\alpha ,\beta )}\Vert _\infty \le 2\) and \(1^{(\epsilon )}_{[\alpha ,\beta )} \rightarrow 1_{[a,b)}\) pointwise for \(\epsilon \rightarrow 0^+\), the Lebesgue dominated convergence theorem and the finiteness of the positive spectral measure \(\mu ^{(\overline{aA+bB})}_{\psi ,\psi }(E):=\langle \psi P^{(\overline{aA+bB})}_E\psi \rangle \) imply that
Since \(P^{(\overline{aA+bB})}_{[\alpha ,\beta )}= 1_{[\alpha ,\beta )}(\overline{aA+bB})\) and on account of the general identity \(\Vert f(\overline{aA+bB})\psi \Vert ^2=\int _{\mathbb R}f(\tau )^2\hbox {d}\mu ^{(\overline{aA+bB})}_{\psi ,\psi }(\tau )\), we have \(P^{(\overline{aA+bB})}_{[\alpha ,\beta )} = \text{ s }\lim _{\epsilon \rightarrow 0^+}1^{(\epsilon )}_{[\alpha ,\beta )} (\overline{aA+bB})\). Moreover, \(1^{(\epsilon )}_{[\alpha ,\beta )}\in {\mathscr {S}}(\mathbb {{{\mathbb {R}}}})\), so that it belongs to \({\mathscr {F}}({\mathbb {R}})\) and we can apply Theorem 2.5 to the righthand side obtaining (38). \(\square \)
Remark 3.2
(1) A statement analogous to that in Theorem 3.1 can be proved for the elements \(P^{(\overline{aA+bB})}_{(\gamma ,\alpha ]}\) with \(\gamma < \alpha \). Knowledge of \(P^{(\overline{aA+bB})}_{(\gamma ,\alpha ]}\) and \(P^{(\overline{aA+bB})}_{[\alpha , \beta )}\) permits one to construct the atom \(P^{(\overline{aA+bB})}_{\{\alpha \}}\) since \(P^{(\overline{aA+bB})}_{(\gamma ,\alpha ]} P^{(\overline{aA+bB})}_{[\alpha , \beta )} = P^{(\overline{aA+bB})}_{(\gamma ,\alpha ] \cap [\alpha , \beta )} = P^{(\overline{aA+bB})}_{\{\alpha \}}\,.\) Alternatively, \(P^{(\overline{aA+bB})}_{\{\alpha \}}\) directly arises from (38) when using \(1^{(\epsilon )}_{\{\alpha \}}(x) := \exp {\{(x\alpha )^2/\epsilon \}}\) in place of \(1^{(\epsilon )}_{[\alpha , \beta )}(x) \).
(2) If \(\alpha \) and \(\beta \) admit corresponding neighborhoods without intersection with the difference \(\sigma (aA+bB) {\setminus } [\alpha , \beta )\), the \(\epsilon \) limit can be removed from the lefthand side of (38) if replacing \(1^{(\epsilon )}_{\{\alpha \}}\) with a map \(1'_{[\alpha , \beta )} \in {\mathcal{D}}({\mathbb {R}})\) which constantly attains the value 1 over \([\alpha , \beta )\) and rapidly vanishes on \(\sigma (aA+bB) {\setminus } [\alpha , \beta )\).
(3) Theorem 3.1 proves that the PVM of \(aA+bB\) can be determined from the PVMs of the operators A and B. With a slightly different approach (assuming \(a=b=1\) for the sake of simplicity), it is also possible to prove a more direct relation between the Fourier transform of the spectral measures \(\mu ^{(\overline{A+B})}_{\psi ,\varphi }\) and those of the spectral measures \(\mu ^{(A)}_{\psi ,\varphi }\) and \(\mu ^{(B)}_{\psi ,\varphi }\). For that, let \(\psi ,\varphi \in {\mathsf {H}}\) and let \(\{\psi _k\}_{k\in {\mathbb {N}}}\subset {\mathsf {H}}\) be a complete orthonormal basis of \({\mathsf {H}}\). From Trotter product formula, it follows that
Together with the injectivity of the Fourier transform for finite measure—c.f. Eq. (16)–(40) provides another (more indirect) relation between \(P^{(\overline{A+B})}\) and \(P^{(A)},P^{(B)}\). Notice that Eq. (40) can be proved without invoking either Lemma 2.2 or Theorem 2.5—although it can be seen as an application of Theorem 2.5 for the case \(f=1_{{\mathbb {R}}}=f_\delta \in {\mathscr {F}}({\mathbb {R}})\), \(\delta \) denoting the Dirac measure centered at 0. \(\square \)
Example 3.3
We provide here an explicit computation of formula (32) which is shown to match with the exact result—c.f. Theorem 2.5 and part (3) Remark 3.2. Let \({\mathsf {H}}=L^2({\mathbb {R}}, \hbox {d}x)\) and let \(A:=X\) be (with obvious domain) the selfadjoint position operator \((X\psi )(x):=x\psi (x)\), and \(B:=P\) the selfadjoint momentum operator (the unique selfadjoint extension of \((B\psi )(x):=i\frac{\hbox {d}\psi }{\hbox {d}x}(x)\) for \(\psi \in {\mathscr {S}}({{\mathbb {R}}})\))^{Footnote 6}. It turns out that \({\mathscr {S}}({{\mathbb {R}}}) \subset D(A)\cap D(B)\) and \(aA+bB\) is essentially selfadjoint thereon for every \(a,b\in {{\mathbb {R}}}\), its closure being a generator of the Weyl algebra [25] according to Stone’s theorem. As a consequence, the previously developed theory can be applied to the pair A,B.
Taking advantage of Weyl algebra commutation relations, namely
we have that for all \(\phi ,\psi \in {\mathsf {H}}\)
We argue that equation (32) reproduces the exact result (41). A simple computation shows that, if \(E\in {\mathscr {B}}({{\mathbb {R}}})\),
for, respectively, \(\psi \in D(A)\) or \(\psi \in D(B)\) and where \({\hat{\cdot }}\) denotes the Fourier–Plancherel transform. With this information, we wish to compute the limit as \(N\rightarrow +\infty \) of
where \(\rho _{\phi ,\psi }(x_1,\ldots ,k_N)=\frac{1}{(2\pi )^{N\frac{1}{2}}}\overline{\phi (x_1)}\prod _{\ell =1}^{N1}\hbox {e}^{ik_{\ell }(x_{\ell +1}x_\ell )}\hbox {e}^{ik_Nx_N}{\widehat{\psi }}(k_N)\). Equality (43) follows from (25) and (42) by applying Fourier–Plancherel transform and its inverse N times. Notice that we can avoid the regularization \(Q_n\) by considering \(\rho \) as a distribution—there is no integration in t. A direct computation leads to
where in the Dirac delta distributions we are ensured that \(x_\ell =x_1\frac{\ell }{N}t\) for \(\ell =2,\ldots , N\). \(\square \)
3.2 Relation with Feynman integration
The next application proves the close relation between formula (32) and the notion of Feynman integral in phase space. Let us consider now a slight modification of Example 3.3. Let \({\mathsf {H}}:=L^2({\mathbb {R}}, \hbox {d}x)\) and let \((A\psi )(x):=x^2\psi (x)\) and \(B:=P^2\) be, respectively, the square of the selfadjoint position and momentum operators defined in Example 3.3. Further let \(a=\Omega ^2 /2\) and \(b=(2m)^{1}\), with \(m,\Omega >0\) constants. It is well known that \(A+B\) is essentially selfadjoint over \({\mathscr {S}}({{\mathbb {R}}}) \subset D(A)\cap D(B)\) and \(\overline{A+B}\) coincides with the harmonic oscillator Hamiltonian operator H
Let us recall that if T is a selfadjoint operator on \({{\mathsf {H}}}\) with spectral measure \(P^{(T)}\) and \(h:{{\mathbb {R}}}\rightarrow {{\mathbb {R}}}\) is a Borel measurable map, the spectral measure \(P^{(h(T))}\) of the selfadjoint operator h(T) (defined via functional calculus out of T) is related to \(P^{(T)}\) by the formula
for any Borelmeasurable function \(f: {{\mathbb {R}}}\rightarrow {{\mathbb {C}}}\).
As a consequence, if \(f\in {\mathscr {F}}({{\mathbb {R}}})\) and using \(h : {{\mathbb {R}}}\ni r \mapsto r^2\), (32) implies
If we now choose the function \(f\in {\mathscr {F}}({{\mathbb {R}}})\) of the form \(f(\lambda )=\hbox {e}^{it\lambda }\), with \(t\in {{\mathbb {R}}}\), then for any \(\phi ,\psi \in {{\mathsf {H}}}\) we have the following representation for the matrix elements of the unitary evolution operator \(U(t)=\hbox {e}^{itH}\)
Analogously to the derivation of equality (43), iterated applications of Fourier transform and its inverse yield
where we recall that the integrals over \({{\mathbb {R}}}^{2N}\) are just a formal symbol standing for the limit of the regularizing procedure described in (25), since in this case the distribution (27) is not associated with a complex measure on \({\mathscr {B}}({{\mathbb {R}}}^{2N})\). Formula (46) admits an interpretation in terms of a phase space Feynman path integral representation for the time evolution operator U(t), as discussed, e.g., in [1, 17]. Indeed, it is possible to look at the exponent appearing in the integral on the righthand side of (46), namely the function
as the Riemann sum approximation of the classical action functional in the Hamiltonian formulation:
where \(h:{{\mathbb {R}}}^2\rightarrow {{\mathbb {R}}}\) is the classical Hamiltonian of the harmonic oscillator, i.e.,
A completely similar discussion can be repeated in the case the harmonic oscillator potential is replaced with a more general potential, namely a measurable map \(V:{{\mathbb {R}}}\rightarrow {{\mathbb {R}}}\) such that the sum of the associated multiplication operator \(M_V:D(M_V)\subset {{\mathsf {H}}}\rightarrow {{\mathsf {H}}}\) and \(B=P^2\) is essentially selfadjoint. We stress that the limit as \(N\rightarrow \infty \) on the righthand side of (46) cannot be interpreted in terms of a welldefined integral over an infinitedimensional space of paths \((q,p):[0,t]\rightarrow {{\mathbb {R}}}^2 \) , formally written (in Feynman path integral notation) as
since it is impossible to construct a corresponding complex measure, as extensively discussed in [2] and in Sect. 4.2.
3.3 (Semi)bounded A, B, Jordan product, polynomials, Feynman–Kac formula
If the selfadjoint operators A and B are bounded, then \(aA+bB \in {{\mathfrak {B}}}({{\mathsf {H}}})\) is defined for all \(a,b \in {\mathbb {R}}\) and (22) permits us to extend (32) to the case of \(f\in C^\infty ({{\mathbb {R}}})\). A similar result is valid when A and B are bounded from below.
Let us start with \(A,B \in {{\mathfrak {B}}}({{\mathsf {H}}})\). For any choice of \(a,b\in {{\mathbb {R}}}\), we then have
for every \(n\in {{\mathbb {N}}}\), if \({\tilde{f}}\in {\mathscr {S}}({{\mathbb {R}}})\) is such that \({\tilde{f}}(x)=f(x)\) if \(x \in [\Vert aA\Vert \Vert bB\Vert , \Vert aA\Vert +\Vert b\Vert ]\). As a consequence, (23) is still valid with \({\tilde{f}}\) in place of f on the righthand side, and the limit does not depend neither on the choice of the regularizing sequence \(Q:=\{Q_n\}_{n\in {{\mathbb {N}}}}\) nor on the choice of \({\tilde{f}}\):
A similar result is found when A and B are (unbounded) selfadjoint operators which are bounded from below and \(a,b \ge 0\) are such that \(aA+bB\) is essentially selfadjoint. In this case \(\overline{aA+bB}\) is bounded from below as well with \(\inf \sigma (\overline{aA+bB}) \ge a\inf \sigma (A) + b \inf \sigma (B)\,.\) With the said A, B, a, b, both (47) and (48) are true provided \(f \in C^\infty ({{\mathbb {R}}})\), \({\tilde{f}} \in {\mathscr {S}}({{\mathbb {R}}})\), and \(f(x) ={\tilde{f}}(x)\) for \(x \ge a\inf \sigma (A) + b \inf \sigma (B)\).
Identity (48) is sufficient in both cases for giving the following definition based on Riesz’ lemma.
Definition 3.4
Assume that one of the following two cases holds
 (a):

\(A,B \in {{\mathfrak {B}}}({{\mathsf {H}}})\) are selfadjoint, \(a,b \in {{\mathbb {R}}}\), and \(f \in C^\infty ({{\mathbb {R}}})\);
 (b):

A, B are selfadjoint and bounded from below, \(a,b\ge 0\), \(aA+bB\) is essentially selfadjoint, and \(f\in C^\infty ({\mathbb {R}})\) is such that there exists \({\tilde{f}}\in {\mathscr {S}}({\mathbb {R}})\) for which \(f(x)={\tilde{f}}(x)\) for \(x\ge a\inf \sigma (A)+b\inf \sigma (B)\).
Then,
is defined as the unique operator satisfying (25). \(\square \)
This definition is an evident extension of the definition for \(f\in {\mathscr {F}}({\mathbb {R}})\) appearing in Theorem 2.3 because, if \({\tilde{f}}\in {\mathscr {S}}({\mathbb {R}})\subset {\mathscr {F}}({\mathbb {R}})\) is defined as above with respect to f, then
The remaining properties (i)–(iv) of Theorem 2.3 hold as well provided \(\Vert f\Vert _{\mathscr {F}}\) is replaced for \(\Vert {\tilde{f}}\Vert _{\mathscr {F}}\) on the righthand side of (26) in (ii).
With this extended definition, Theorem 2.5 is still valid as the reader immediately proves noticing in particular that from (3) and (4), we have
Proposition 3.5
If either (a) or (b) in Definition 3.4 is valid, then
If with \(A,B\in {{\mathfrak {B}}}({{\mathsf {H}}})\), Definition 3.4 applies in particular to the operator \(aA+bB\) as in (51) below, when referring to the smooth map \(f: {{\mathbb {R}}}\ni x \mapsto x \in {{\mathbb {R}}}\). That identity shows how the real linear space structure of the algebra of bounded observables can be constructed employing the PVMs of the involved observables only. The whole algebra of bounded observables \({{\mathfrak {B}}}({{\mathsf {H}}})\) has another natural operation that is the (nonassociative) Jordan product:
The Jordan product of A and B admits an expansion similar to (51) where, again, only the PVMs of A and B is used. These results can be further generalized as stated in the last item of the following theorem which concerns polynomials.
Theorem 3.6
Let \(A, B\in {{\mathfrak {B}}}({{\mathsf {H}}})\) be selfadjoint operators, with \({{\mathsf {H}}}\) separable, whose PVMs are, respectively, denoted by \(P^{(A)}\) and \(P^{(B)}\). Let \(\nu ^{(N,n)}_{\phi ,\psi ,Q} :{\mathscr {B}}({{\mathbb {R}}}^{2N})\rightarrow {{\mathbb {C}}}\) be the complex measures defined as in (21). The following facts are true.
 (a):

If \(a,b \in {{\mathbb {R}}}\),
$$\begin{aligned} aA+bB = \text{ s }\lim _{N\rightarrow +\infty } \int _{{{\mathbb {R}}}^{2N}} \left( a\sum ^N_{n=1} \frac{\lambda _n}{N} + b\sum ^N_{n=1} \frac{\mu _n}{N} \right) \, \mathrm{d}P^{(A)}_{\lambda _1}\mathrm{d}P^{(B)}_{\mu _1}\cdots \mathrm{d}P^{(A)}_{\lambda _N}\mathrm{d}P^{(B)}_{\mu _N}\,. \end{aligned}$$(51)  (b):

The Jordan product of A and B satisfies
$$\begin{aligned} A\circ B = {s}\lim _{N\rightarrow +\infty } \int _{{{\mathbb {R}}}^{2N}} \left( \sum ^N_{n=1} \frac{\lambda _{n}}{N}\right) \left( \sum ^N_{n=1} \frac{\mu _{n}}{N}\right) \,\, \mathrm{d}P^{(A)}_{\lambda _1}\mathrm{d}P^{(B)}_{\mu _1}\cdots \mathrm{d}P^{(A)}_{\lambda _N}\mathrm{d}P^{(B)}_{\mu _N}\,, \end{aligned}$$(52)where the operator after the symbol of limit is the unique operator such that
$$\begin{aligned}&\left\langle \phi \left \int _{{{\mathbb {R}}}^{2N}}\left( \sum ^N_{n=l} \frac{\lambda _{l}}{N}\right) \left( \sum ^N_{n=l} \frac{\mu _{l}}{N}\right) \,\,\mathrm{d}P^{(A)}_{\lambda _1}\mathrm{d}P^{(B)}_{\mu _1}\cdots \mathrm{d}P^{(A)}_{\lambda _N}\mathrm{d}P^{(B)}_{\mu _N}\psi \right. \right\rangle \nonumber \\&\quad =\lim _{n\rightarrow \infty } \int _{{{\mathbb {R}}}^{2N}} \left( \sum _{l=1}^{N}\frac{\lambda _l}{N}\right) \left( \sum _{l=1}^{N}\frac{\mu _l}{N}\right) \,\, \mathrm{d}\nu ^{(N,n)}_{\phi ,\psi ,Q}(\lambda _1, \mu _1, \dots , \lambda _N,\mu _N)\,, \end{aligned}$$(53)for all \(\phi , \psi \in {{\mathsf {H}}}\).
 (c):

Assume \(p,q=0,1,2,\ldots \) and let \(S_{p+q}(A^p B^q)\) denote the selfadjoint operator consisting of the symmetrized product of p copies of A and q copies of B,
$$\begin{aligned} S_{p+q}(A^p B^q) := {p+q\atopwithdelims ()q}^{1}(A^pB^q+ A^{p1}BAB^{q1}+ \cdots + B^qA^p)\,. \end{aligned}$$If only a finite number of coefficients \(c_{p,q}\in {{\mathbb {R}}}\) do not vanish, then
$$\begin{aligned}&\sum _{p,q} c_{p,q}S_{p+q}(A^p B^q) \nonumber \\&\quad = \text{ s }\lim _{N\rightarrow +\infty } \int _{{{\mathbb {R}}}^{2N}} \sum _{p,q} c_{p,q}\left( \sum ^N_{n=1} \frac{\lambda _{n}}{N}\right) ^p \left( \sum ^N_{n=1} \frac{\mu _{n}}{N}\right) ^q \,\, \mathrm{d}P^{(A)}_{\lambda _1}\mathrm{d}P^{(B)}_{\mu _1}\cdots \mathrm{d}P^{(A)}_{\lambda _N}\mathrm{d}P^{(B)}_{\mu _N}\,, \end{aligned}$$(54)where the operator after the symbol of limit is the unique operator such that
$$\begin{aligned}&\left\langle \phi \left \int _{{{\mathbb {R}}}^{2N}}\sum _{p,q} c_{p,q}\left( \sum ^N_{l=1} \frac{\lambda _{l}}{N}\right) ^p \left( \sum ^N_{l=1} \frac{\mu _{l}}{N}\right) ^q \,\,\mathrm{d}P^{(A)}_{\lambda _1}\mathrm{d}P^{(B)}_{\mu _1}\cdots \mathrm{d}P^{(A)}_{\lambda _N}\mathrm{d}P^{(B)}_{\mu _N}\psi \right. \right\rangle \nonumber \\&\quad =\lim _{n\rightarrow \infty } \int _{{{\mathbb {R}}}^{2N}} \sum _{p,q} c_{p,q}\left( \sum _{l=1}^{N}\frac{\lambda _l}{N}\right) ^p\left( \sum _{l=1}^{N}\frac{\mu _l}{N}\right) ^q\,\, \mathrm{d}\nu ^{(N,n)}_{\phi ,\psi ,Q}(\lambda _1, \mu _1, \dots , \lambda _N,\mu _N)\,,\nonumber \\ \end{aligned}$$(55)for all \(\phi , \psi \in {{\mathsf {H}}}\).
The limit in the righthand side of (53) and (55) does not depend on the choice of the regularizing sequence Q.
Proof
We only have to prove (b) and (c). Regarding (b), it essentially relies on the elementary decomposition \(xy = \frac{1}{2}(x+y)^2\frac{1}{2}x^2\frac{1}{2}y^2\), which implies
As discussed above, the limits for \(n\rightarrow +\infty \) of the final three addends exist and do not depend on the used sequence Q. We conclude that the righthand side of (53) exists and does not depend on Q. More precisely, from (48),
where \({\tilde{f}}:{{\mathbb {R}}}\rightarrow {{\mathbb {R}}}\) is such that \({\tilde{f}}\in {\mathscr {S}}({{\mathbb {R}}})\) such that \({\tilde{f}}(x) = x^2\) for the values \(x \in [\Vert A\Vert \Vert B\Vert , \Vert A\Vert +\Vert B\Vert ]\). At this point, Riesz’ lemma proves that there is a unique operator satisfying (53). Decomposing
on the righthand side of (52), and noticing that analogously to \(xy = \frac{1}{2}(x+y)^2\frac{1}{2}x^2\frac{1}{2}y^2\),
(52) is an immediate consequence of (50) applied to the three addends on the righthand sides of the two identities above. The proof of (c) is a straightforward generalization the proof of (b). It relies on the wellknown Sylvester’s result (see, e.g., the review part of [32]), that every real (or complex) homogeneous polynomial in x and y of degree m, in particular the monomial \(x^py^q\) (with \(m:=p+q)\), can be decomposed as \(x^py^q = \sum _{k} (a_kx+b_ky)^m\) for a finite number (\(\le m+1\)) of constants \(a_k,b_k \in {{\mathbb {R}}}\) (resp. \({{\mathbb {C}}}\)), and the fact that this result easily implies \(S_{p+q}(A^pB^q) = \sum _k (a_kA+b_kB)^m\). \(\square \)
Remark 3.7
Item (c) proves the existence of a linear map associating each real polynomial p on \({{\mathbb {R}}}^2\) to a suitably symmetrized (as in the lefthand side of (54)) polynomial of the operators A and B. One naturally wonders if that map is a quantization map [18]. It is not possible to answer the question without further information on the \(^*\)algebra generated by A and B. As a matter of fact, a necessary condition is that the aforementioned map transforms a Poisson structure on the space of polynomials to a real Liealgebra structure on the space of the said polynomials of A and B, whose Lie bracket is the commutator of operators (more precisely \(i[\cdot , \cdot ]\)). In the general case, the space of those polynomials of operators is not a Lie algebra, unless A and B satisfy some further relations, in particular, it must be possible to expand i[A, B] as a real polynomial of A and B which is symmetrized as said. \(\square \)
Case (b) in Proposition 3.5 has an interesting application which proves the interplay of formula (32) and the socalled Feynman–Kac formula.
Example 3.8
Let us consider again the setting of Sect. 3.2. Since in this case both operators A and B have positive spectrum, we can apply formula (50) also for f with exponential growth. In particular, we can choose \(f:{{\mathbb {R}}}\rightarrow {{\mathbb {R}}}\) of the form \(f(\lambda )=\hbox {e}^{\tau \lambda }\), with \(\tau > 0\), obtaining the following representation for the matrix elements of the semigroup generated by the selfadjoint operator H [see Eq. (44)]:
If \(\psi \in L^1({{\mathbb {R}}},\hbox {d}x)\), the integrals on \({{\mathbb {R}}}^{2N+1}\) appearing on the righthand side are absolutely convergent thanks to the fast decaying properties of the exponentials appearing in the integrand. In particular, in this case, by applying Fubini theorem and integrating with respect to \(k_1,\ldots , k_N\), we get
In this case, thanks to the presence of the Gaussian density
in the integrand, the limit for \(N\rightarrow \infty \) of the finitedimensional integrals appearing in the righthand side of (59) can be interpreted in terms of an integral over the Banach space \(C_\tau ({{\mathbb {R}}})\) of continuous paths \(\omega :[0,\tau ]\rightarrow {{\mathbb {R}}}\) endowed with the uniform norm, the corresponding Borel \(\sigma \)algebra and the Wiener Gaussian measure W. By a standard argument (see, e.g., [38]), formula (59) yields the celebrated Feynman–Kac formula:
As remarked at the end of Sect. 3.2, the discussion above generalizes to the case the harmonic oscillator potential is replaced with a Borel measurable nonnegative map \(V:{{\mathbb {R}}}\rightarrow {{\mathbb {R}}}\) such that the sum of the associated multiplication operator \(M_V:D(M_V)\subset {{\mathsf {H}}}\rightarrow {{\mathsf {H}}}\) and \(B=P^2\) is essentially selfadjoint. Related ideas can be also found in [15, 16, 29] as well as in Lapidus’ papers from the late 1980s [19,20,21]. \(\square \)
4 Counterexamples
In this section, we provide a series of counterexamples which make evident the rigidity of the structures involved in the rigorous generalization of formula (8) to infinitedimensional case—c.f. Theorem 2.5.
In Sect. 2, we introduce a regularization procedure through the projectors \(Q_n\) to safely define a family of measures \(\nu ^{(N,n)}_{\phi ,\psi }\) whose distributional limit \(n\rightarrow +\infty \) permitted us to define the operator integral in Eq. (24)—c.f. Theorem 2.3. This may appear artificial at first glance and one may wonder if the regularization \(Q_n\) can be removed. This is not the case—c.f. Sect. 4.1.
Moreover, even in the finitedimensional case—where \(Q_n\) can be chosen to be the identity and \(\nu ^{(N)}_{\phi ,\psi }\) does exists as a complex measure on \({\mathbb {R}}^{2N}\)—the properties of the sequence of measures \(\lbrace \nu ^{(N)}_{\phi ,\psi }\rbrace _N\) are, however, not sufficient to define a suitable projective limit \(N\rightarrow +\infty \)—c.f. Sect. 4.2.
Finally, the convergence properties of \(\mu ^{(N,n)}_{\phi ,\psi }\) as \(n\rightarrow +\infty \) are considered in the best case scenario, namely when \(P^{(A)}\), \(P^{(B)}\) commute. Even in this, in a sense tamed situation, simple cases pop out where \(\mu ^{(N,n)}_{\phi ,\psi }\) does not converge in the space of complex measure \({\mathscr {M}}({\mathbb {R}}^{2N})\)—c.f. Sect. 4.3.
4.1 The \(Q_n\)regularization is generally necessary
Lemma 2.2 introduces the regularized measure \(\nu ^{(N,n)}_{\phi ,\psi }\) which is built out of the PVMs \(P^{(A)}\), \(P^{(B)}\) associated with the operators A, B together with a suitable “regularizing” sequence of projectors \(\{Q_n\}\). One may wonder whether it is possible to avoid the regularization \(\{Q_n\}\), thus considering a complex measure \(\nu ^{(N)}_{\phi ,\psi }\) defined on products of Borel set \(I_\ell ,J_\ell \in {\mathscr {B}}({\mathbb {R}})\) as
Unfortunately, \(\nu ^{(N)}_{\phi ,\psi }\) generally does not extend to a complex measure on \({\mathbb {R}}^{2N}\) as is in particular shown by the following physically relevant example.
Example 4.1
With reference to Example 3.3, let us check if, in this concrete case, \(\nu ^{(N)}_{\phi ,\psi }\) extends to a complex measure on \({\mathbb {R}}^{2N}\).
For all \(I_1,J_1,\ldots ,I_N,J_N\in {\mathscr {B}}({\mathbb {R}})\), we have
Since \(\rho _{\phi ,\psi }\in L^1_{\mathrm {loc}}({\mathbb {R}}^{2N},d^Nxd^Nk){\setminus } L^1({\mathbb {R}}^{2N},d^Nxd^Nk)\), it is evident that \(\nu ^N_{\phi ,\psi }\) does not extend to a welldefined complex measure on \({\mathbb {R}}^{2N}\) because the total variation of such complex measure would be \(\rho _{\phi ,\psi }_{L^1({\mathbb {R}}^{2N},d^Nxd^Nk)}\) which is not finite. \(\square \)
4.2 The sequence of measures \(\nu ^{(N)}_{\phi ,\psi }\) generally does not admit a (projective) limit
Let us consider the elementary case of a finitedimensional Hilbert space, where the regularization driven by Q is not necessary. In fact, we can simply fix \(Q_n = I\).
A natural issue is whether or not it is possible to interpret the limit for \(N\rightarrow \infty \) on the righthand side of (8) in terms of a integral on an infinitedimensional space. Indeed, in the particular case where \({{\mathsf {H}}}\) is finite dimensional, for any \(\phi ,\psi \in {{\mathsf {H}}}\) it is possible to define a family of complex Borel measures \(\{\nu ^{(N)}_{\phi ,\psi }\}_{N\in {\mathbb {N}}}\), with \(\nu ^{(N)}_{\phi ,\psi }:{\mathscr {B}}({{\mathbb {R}}}^{2N})\rightarrow {{\mathbb {C}}}\). By introducing for any \(M,N\in {{\mathbb {N}}}\) with \(M\le N\), the projection maps \(\pi ^N_M:{{\mathbb {R}}}^{2N}\rightarrow {{\mathbb {R}}}^{2M}\), it is simple to see that the measures \(\{\nu ^{(N)}_{\phi ,\psi }\}_{N\in {\mathbb {N}}}\) fulfill the consistency condition
that is, for all \(I_1,\ldots ,I_M, J_1,\ldots ,J_M\in {\mathscr {B}}({{\mathbb {R}}})\)
It is then meaningful to investigate whether the projective family of complex measures \(\{\nu ^{(N)}_{\phi ,\psi }\}_{N\in {\mathbb {N}}}\) admits a projective limit. For that, let us consider the infinitedimensional space \(({{\mathbb {R}}}\times {{\mathbb {R}}})^{{\mathbb {N}}}\) of all sequences \(\{(\lambda _n,\mu _n)\}_{n \in {\mathbb {N}}}\). Moreover, let \(\Sigma \) be the \(\sigma \)algebra on \(({{\mathbb {R}}}\times {{\mathbb {R}}})^{{\mathbb {N}}}\) generated by the cylinder sets \(\pi _N^{1}(E)\), where \(N\in {\mathbb {N}}\), \(E\in {\mathscr {B}}({{\mathbb {R}}}^{2N})\) and \(\pi _N:({{\mathbb {R}}}\times {{\mathbb {R}}})^{{\mathbb {N}}}\rightarrow ({{\mathbb {R}}}\times {{\mathbb {R}}})^N\) is the canonical projection map. Within this setting, it is meaningful to investigate the existence of a complex bounded measure \(\nu _{\phi ,\psi }\) on \(( ({{\mathbb {R}}}\times {{\mathbb {R}}})^{{\mathbb {N}}}, \Sigma )\) such that \(\nu ^{(N)}_{\phi ,\psi }=(\pi _N)_*\nu _{\phi ,\psi } \) for all \(n\in {{\mathbb {N}}}\) (see “3” for further details). However, as proved in “3,” a necessary condition for the existence of \(\nu _{\phi , \psi }\) is a uniform bound on the total variation \(\Vert \nu ^{(N)}_{\phi ,\psi }\Vert =\nu ^{(N)}_{\phi ,\psi }({\mathbb {R}}^{2N})\) of the measures \(\{\nu ^{(N)}_{\phi ,\psi }\}_{N\in {\mathbb {N}}}\). Unfortunately, in general this does not hold when A and B do not commute as the following example shows.
Example 4.2
Let us consider the special case \({{\mathsf {H}}}={{\mathbb {C}}}^2\), where \(A:=\sigma _z\) and \(B:=\sigma _x\), \(\sigma _z, \sigma _x\) denoting two Pauli matrices. In this case, the Hilbert space is finite dimensional and for any \(N\ge 1\) and \(\phi , \psi \in {{\mathbb {C}}}^2\), it is possible to define the complex Borel measure \(\nu ^N_{\phi , \psi }\) on \(\{\pm 1\}^{2N}\) (the topology being the discrete one) as:
where \(a_1,\ldots ,a_N, b_1,\ldots , b_N\in \{\pm 1\}\) and \(P^{(A)}_{\pm }, P^{(B)}_{\pm }\) are defined as
where \(z_+\rangle , z_\rangle \), resp.\(x_+\rangle , x_\rangle \), are the normalized eigenvectors of \(\sigma _z\), resp. \(\sigma _x\).
The total variation of \(\nu ^{(N)}_{\phi , \psi }\) can be computed explicitly here. Indeed, by writing the vectors \(\phi , \psi \) as linear combinations of the vectors of the orthonormal basis \( \{z_+\rangle , z_\rangle \}\) and \( \{x_+\rangle , x_\rangle \}\), namely:
we get for any \((a_1,b_1,\ldots ,a_N,b_N)\in \{\pm 1\}^{2N}\):
Hence, we obtain
The sequence of measures \(\nu ^{(N)}_{\phi ,\psi }\) cannot admit a projective limit, since \(\sup _N \left \nu ^{(N)}_{\phi , \psi }\right =+\infty \). \(\square \)
The illustrated nogo result is strictly related to the noncommutativity of the spectral projectors \(P^{(A)}\) and \(P^{(B)}\). In fact, in the general case of a separable Hilbert space \({{\mathsf {H}}}\), if the spectral measures \(P^{(A)}\) and \(P^{(B)}\) commute then, for any couple of normalized vectors \(\phi , \psi \in {{\mathsf {H}}}\) and for any \(N\ge 1\), the formula
defines a complex measure with finite total variation. In particular, since
the following identity holds for any set \(E\in {\mathscr {B}}({{\mathbb {R}}}^{2N})\),
where \(\nu ^{(1)}_{\phi , \psi }(I\times J)=\langle \phi  P^{(A)}_{I}P^{(B)}_{J}\psi \rangle \) is associated with the joint spectral measure of A and B. By (60), it is simple to obtain the following inequality for any \(N\ge 1\)
In addition, in the particular case where \(\phi =\psi \) and \(\Vert \phi \Vert =1\) formula (8) admits a simple probabilistic interpretation. Indeed, in this case the measures \(\{\nu ^{(N)}_{\phi , \psi }\}_N\) form a consistent family of probability measures that can be interpreted as the joint distributions of a sequence \(\{\xi _n,\eta _n\}_n\) of random variables with values in \({{\mathbb {R}}}^2\) which are in fact trivially completely correlated, i.e., \((\xi _n,\eta _n)=(\xi _1,\eta _1)\) for all \(n\in {{\mathbb {N}}}\), and the distribution of the random vector \((\xi _1,\eta _1)\) is given by the joint spectral measure of A and B.
In the case the commutativity condition is not fulfilled, then a uniform bound as (61) cannot be obtained in general as the following example shows.
Example 4.3
Let us consider again \({{\mathsf {H}}}:={{\mathbb {C}}}^2\) as before, and the two spectral measures \(P^{(A)}\) and \(P^{(B)}\) on \(\{\pm \, 1\}\) defined as
where
Let us choose \(\phi :=\frac{\sqrt{2}}{2} z_+\rangle +\frac{\sqrt{2}}{2} z_\rangle \) and \(\psi :=\frac{\sqrt{2}}{2} v_+\rangle +\frac{\sqrt{2}}{2} v_\rangle \) and consider again the complex measure \(\nu ^{(N)}_{\phi , \psi }\) on \(\{\pm 1\}^{2N}\) defined for any \((a_1,b_1,\ldots ,a_N,b_N)\in \{\pm 1\}^{2N}\) by
It is simple to verify that
which shows that \(\sup _N\nu ^{(N)}_{\phi , \psi }=+\infty \), unless the spectral measures commute. \(\square \)
4.3 Convergence of \(\{\mu ^{(N,n)}_{\phi ,\psi }\}_{n \in {\mathbb {N}}}\) in \({\mathscr {M}}({\mathbb {R}}^{2N})\) for commuting PVMs: a counterexample
Let us consider once again the sequence of finite complex measure \(\nu ^{(N,n)}_{\phi ,\psi }\) on \({\mathbb {R}}^{2N}\). Since \(Q_n\rightarrow I\), strongly it follows that for all \(I_\ell ,J_\ell \in {\mathscr {B}}({\mathbb {R}}^N)\),
Unfortunately, as shown in Example 4.1, \(\nu ^{(N)}_{\phi ,\psi }\) does not define a measure on \({\mathbb {R}}^{2N}\). However, whenever \([P^{(A)},P^{(B)}]=0\), \(\nu ^{(N)}_{\phi ,\psi }\) does define a complex measure on \({\mathbb {R}}^{2N}\)—c.f. Sect. 4.2. Therefore, one may wonder whether the convergence \(\nu ^{(N,n)}_{\phi ,\psi }\rightarrow \nu ^{(N)}_{\phi ,\psi }\) holds true in the space of complex measure \({\mathscr {M}}({\mathbb {R}}^{2N})\), namely if
Unfortunately, this is not the case as shown in particular by the following example.
Example 4.4
Let us consider \({\mathsf {H}}=L^2([0,1],\hbox {d}x)\) and let \(A=B=X\) be the usual position operator over [0, 1]–c.f. Example 4.1. We consider the complete orthonormal basis \(\{e_k\}_{k\in {\mathbb {Z}}}\) of \(L^2([0,1],\hbox {d}x)\) made by exponentials \(e_k(x):=\hbox {e}^{2\pi ikx}\) and we set \(Q_n:=\sum _{k\le n} e_k\rangle \langle e_k\) for \(n\in {\mathbb {N}}\). Moreover, we choose \(\psi =\phi =1_{[0,1]}\in L^2([0,1],\hbox {d}x)\). It follows that for all \(I,J\in {\mathscr {B}}([0,1])\) (where the Borel algebra is referred to the topology on [0, 1] form \({\mathbb {R}}\)),
where \( \rho _n(xy):=\sum _{k\le n}e_k(xy)\). A direct computation yields \(\Vert \nu ^{(1)}_{\phi ,\psi }\Vert =\nu ^{(1)}_{\phi ,\psi }([0,1]^2)=1\) while \(\Vert \nu ^{(1,n)}_{\phi ,\psi }\Vert =\Vert \rho _n\Vert _{L^1([0,1],\hbox {d}x)}\). Since the linear map \(L^1([0,1],\hbox {d}x)\ni f\mapsto m_f\in {\mathscr {M}}([0,1]^2)\)—defined by \(m_f(E):=\int _E f(xy)\hbox {d}x\hbox {d}y\)—is a (nonsurjective) isometry and both spaces are complete, it follows that convergence of \(\nu ^{(1,N)}_{\psi ,\psi }\) in \({\mathscr {M}}([0,1]^2)\) would imply convergence of \(\rho _n\) in \(L^1([0,1],\hbox {d}x)\) to some function therein. However, this is impossible since \(\rho _n\) weakly converges to the Dirac delta \(\delta \) centered at 0 which cannot be represented by a function of \(L^1([0,1],\hbox {d}x)\). \(\square \)
5 Toward a physical interpretation
In the particular case where the Hilbert space \({{\mathsf {H}}}\) is finite dimensional and no technical issues must be addressed, it is interesting to discuss the physical interpretations of formula (8).
To this end, we recall that if, as assumed, the Hilbert space is separable with \(\dim ({{\mathsf {H}}}) \ne 2\), the Gleason theorem [8, 11] establishes that quantum states viewed as \(\sigma \)additive measures \(\mu \) on \({\mathcal {L}}({\mathsf {H}})\) are onetoone with positive, traceclass, unittrace operators \(\rho _\mu : {{\mathsf {H}}}\rightarrow {{\mathsf {H}}}\). Pure states are the extremal elements \(\nu \) of the convex body of states and they are in a onetoone correspondence with unit vectors \(\psi _\nu \) up to phases and \(\nu (P)=P\psi _\nu ^2\) is the probability that \(P\in {\mathscr {L}}({{\mathsf {H}}})\) is true if the pure state is represented by \(\psi _\nu \).
5.1 Noncommutativity and quantum interference terms
We start the analysis with the following elementary observation. Since the identity operator can be decomposed either as \(I=\sum _{\lambda \in \sigma (A)}P^{(A)}_\lambda \) or as \(I=\sum _{\mu \in \sigma (B)}P^{(B)}_\mu \), for any \(N\in {{\mathbb {N}}}\) and \(\psi \in {{\mathsf {H}}}\) we have
Above, the state vector \(\psi \) is decomposed into a coherent superposition of generally nonmutually orthogonal vector states. These vectors would be mutually orthogonal if the PVMs commuted. The presence in (8) of these nonorthogonal vectors is the source of a quantum interference phenomenon we are going to illustrate.
The weak version of formula (8) reads as follows:
for any \(\phi , \psi \in {{\mathsf {H}}}\). In particular, when \(\phi =\psi \), we get
As usual, the lefthand side coincides with the expectation value of the observable \(f(aA+bB)\) when the state is pure and represented by the unit vector \(\psi \). In particular, if \(f=1_{[\alpha , \beta )}\) [in this case (64) should be replaced by (14)], the lefthand side is nothing but the probability of obtaining an outcome in \([\alpha ,\beta )\) when measuring \(aA+bB\) over the pure state represented by the unit vector \(\psi \).
Exploiting (62) in the expansion the left entry of the inner products, formula (64) can be rephrased to
where we defined \(({{\bar{\lambda }}}, {{\bar{\mu }}}):=(\lambda _1,\ldots , \lambda _N, \mu _1,\ldots , \mu _N)\) and \( (\overline{\tilde{\lambda }},\overline{{{\tilde{\mu }}}}):=({{\tilde{\lambda }}} _1,\ldots , {{\tilde{\lambda }}} _N, {{\tilde{\mu }}} _1, \ldots , {{\tilde{\mu }}} _N)\).
The considered expectation value is therefore tantamount to the sum two distinct kinds of terms.

(1)
The first type admits to some extent (see (1) Remark 5.1) a “classical” probabilistic interpretation relying on a recursive use of Born’s rule and the standard Lüders–von Neumann’s postmeasurement state postulate (see, e.g., [4, 18, 25]). As is well known, the former postulate states that if the initial pure states are represented by the unit vector \(\psi \in {{\mathsf {H}}}\), the probability that the outcome of an elementary YES–NO observable \(P\in {\mathscr {L}}({{\mathsf {H}}})\) is 1 (YES) is \(P\psi ^2\). The latter postulate says that if the outcome resulted to be 1, then the postmeasurement state is represented by the normalized vector \(P\psi ^{1}P\psi \). As a matter of fact, the positive number
$$\begin{aligned} \Vert P^{(A)}_{\lambda _1} P^{(B)}_{\mu _1}\cdots P^{(A)}_{\lambda _N} P^{(B)}_{\mu _N}\psi \Vert ^2\in [0,1] \end{aligned}$$can be interpreted as a conditional probability^{Footnote 7}: the probability that, given the initial pure state of the system described by the normalized vector \(\psi \in {{\mathsf {H}}}\), in a sequence of 2N measurements of observables \(O_j\), \(J=1,\ldots ,2N\), with \(O_j=B\) for j odd and \(O_j=A\) for j even, the sequence of outcomes is exactly \((\mu _N, \lambda _N,\ldots , \mu _1, \lambda _1)\). Let us illustrate this point in some detail. Given a general observable O in our finitedimensional Hilbert space with (necessarily discrete) spectrum \(\sigma (O)\), and a normalized vector \(\phi \in {{\mathsf {H}}}\), we shall denote with the symbol \({{\mathbb {P}}}(O=o\phi ) \) the probability that, given that the (pure) state of the system is represented by \(\phi \), the outcome of the measurement of O is the real number \(o\in \sigma (O)\), namely
$$\begin{aligned} {{\mathbb {P}}}(O=o\phi )= P^{(O)}_o\phi ^2, \end{aligned}$$where \(P^{(O)}_o\) is the spectral projector associated with the eigenvalue \(o\in \sigma (O)\). Let us denote by \(\psi _{\lambda _j, \mu _j, \lambda _{j+1},\dots , \lambda _N, \mu _N}\) and \(\psi _{ \mu _j, \lambda _{j+1},\mu _{j+1},\dots , \lambda _N, \mu _N}\) the postmeasurement normalized vectors
$$\begin{aligned} \psi _{\lambda _j, \mu _j, \lambda _{j+1},\dots , \lambda _N, \mu _N}:= & {} \frac{P^{(A)}_{\lambda _j}P^{(B)}_{ \mu _j}P^{(A)}_{ \lambda _{j+1}}\cdots P^{(A)}_{ \lambda _N} P^{(B)}_{ \mu _N}\psi }{\Vert P^{(A)}_{\lambda _j}P^{(B)}_{ \mu _j}P^{(A)}_{ \lambda _{j+1}}\cdots P^{(A)}_{ \lambda _N}P^{(B)}_{ \mu _N}\psi \Vert },\\ \psi _{ \mu _j, \lambda _{j+1},\mu _{j+1},\dots , \lambda _N, \mu _N}:= & {} \frac{P^{(B)}_{ \mu _j}P^{(A)}_{ \lambda _{j+1}}P^{(A)}_{ \mu _{j+1}}\cdots P^{(A)}_{ \lambda _N}P^{(B)}_{ \mu _N}\psi }{\Vert P^{(B)}_{ \mu _j} P^{(A)}_{ \lambda _{j+1}}P^{(A)}_{ \mu _{j+1}}\cdots P^{(A)}_{ \lambda _N}P^{(B)}_{ \mu _N}\psi \Vert } , \end{aligned}$$with \(j=1,\ldots ,N\). We then have:
$$\begin{aligned}&\Vert P^{(A)}_{\lambda _1}P^{(B)}_{\mu _1}\cdots P^{(A)}_{\lambda _N} P^{(B)}_{\mu _N}\psi \Vert ^2 ={{\mathbb {P}}}(A=\lambda _1\psi _{ \mu _1, \lambda _{2},\dots , \lambda _N, \mu _N}) \Vert P^{(B)}_{\mu _1}\cdots P^{(A)}_{\lambda _N} P^{(B)}_{\mu _N}\psi \Vert ^2\\&\quad ={{\mathbb {P}}}(A=\lambda _1\psi _{ \mu _1, \lambda _{2},\dots , \lambda _N, \mu _N}) {{\mathbb {P}}}(B=\mu _1\psi _{ \lambda _{2},\mu _2 ,\dots , \lambda _N, \mu _N}) \Vert P^{(A)}_{\lambda _2}P^{(B)}_{\mu _2}\cdots P^{(A)}_{\lambda _N} P^{(B)}_{\mu _N}\psi \Vert ^2\,. \end{aligned}$$By induction over N, we get the wanted result:
$$\begin{aligned}&\Vert P^{(A)}_{\lambda _1} P^{(B)}_{\mu _1}\cdots P^{(A)}_{\lambda _N} P^{(B)}_{\mu _N}\psi \Vert ^2\nonumber \\&\quad =\Pi _{j=1}^{N1}{{\mathbb {P}}}(A=\lambda _j\psi _{ \mu _j, \lambda _{j+1},\dots , \lambda _N, \mu _N}){{\mathbb {P}}}(B=\mu _j\psi _{ \lambda _{j+1},\mu _{j+1} ,\dots , \lambda _N, \mu _N})\nonumber \\&\qquad \cdot {{\mathbb {P}}}(A=\lambda _N\psi _{\mu _N}){{\mathbb {P}}}(B=\mu _N\psi )\,. \end{aligned}$$(66)It is now evident that the righthand side has the natural interpretation as the probability that, given the initial pure state of the system described by the normalized vector \(\psi \in {{\mathsf {H}}}\), in a sequence of 2N measurements of observables \(O_j\), \(J=1,\ldots ,2N\), with \(O_j=B\) for j odd and \(O_j=A\) for j even, the sequence of outcomes is exactly \((\mu _N, \lambda _N,\ldots , \mu _1, \lambda _1)\).

(2)
The remaining terms appearing in the last line of Eq. (65) are of the form
$$\begin{aligned} \langle P^{(A)}_{{{\tilde{\lambda }}}_1} P^{(B)}_{{{\tilde{\mu }}}_1}\cdots P^{(A)}_{{{\tilde{\lambda }}}_N} P^{(B)}_{{{\tilde{\mu }}}_N}\psi  P^{(A)}_{\lambda _1} P^{(B)}_{\mu _1}\cdots P^{(A)}_{\lambda _N} P^{(B)}_{\mu _N}\psi \rangle , \end{aligned}$$(67)with \( ({{\tilde{\lambda }}}_1,\ldots , {{\tilde{\mu }}}_{N})\ne (\lambda _1,\ldots , \mu _N)\) being complex numbers which can be interpreted as quantum amplitudes or interference terms arising from the coherent decomposition (62) into nonorthogonal addends. In the trivial case where the spectral measures \(\{P^{(A)}_\lambda \}_{\lambda \in \sigma (A)}\) and \(\{P^{(B)}_\mu \}_{\mu \in \sigma (B)}\) commute, it is easy to check that all the interference terms (67) vanish as already remarked. In this sense, their presence has an evident quantum nature.
Remark 5.1
(1) It is worth stressing that also the quantum conditional probability discussed in (1) enjoys different properties than those of the classical conditional probability when the PVMs do not commute. This is because we are here dealing with the quantum notion of probability characterized by Gleason’s theorem, defined on a orthomodular lattice rather than a \(\sigma \)algebra. In particular, the classical identity \({{\mathbb {P}}}(UV){{\mathbb {P}}}(V) = {{\mathbb {P}}}(VU){{\mathbb {P}}}(U)\) has not a corresponding version at quantum level when U and V are replaced for quantum incompatible events. This is reflected from the fact that the order in the sequence of measurements \(P^{(B)}_{\mu _1}\cdots P^{(A)}_{\lambda _N} P^{(B)}_{\mu _N}\) cannot be ignored.
(2) If \({{\mathsf {H}}}\) is finite dimensional, we have the following limit in the operator norm
We now provide an expansion of \(f_N(A,B)\) in terms of spectral commutators of A and B which highlights the link between noncommutativity of spectral measures and appearance of terms of second kind in the righthand side of (65). For that let \(C_{\lambda ,\mu }:=[P^{(A)}_\lambda ,P^{(B)}_\mu ]\) and set \(\wp _N(\lambda _1,\ldots ,\lambda _N;\mu _1,\ldots ,\mu _N):=P^{(A)}_{\lambda _1}P^{(B)}_{\mu _1}\cdots P^{(A)}_{\lambda _N}P^{(B)}_{\mu _N}\). A direct computation leads to
where we set \(\Delta _{\lambda _\ell ,\lambda _{\ell +1}}=\delta _{\lambda _\ell ,\lambda _{\ell +1}}\) for \(1\le \ell <N\), \(\delta _{i,j}\) denoting the Kronecker symbol, while \(\Delta _{\lambda _N,\lambda _{N+1}}=P^{(A)}_{\lambda _N}\). Notice that the product of the terms \(P^{(B)}_{\mu _\ell }\Delta _{\lambda _\ell ,\lambda _{\ell +1}}\) provides the contribution arising from the classical convolution formula, namely \(\prod _{\ell =1}^NP^{(B)}_{\mu _\ell }\Delta _{\lambda _\ell ,\lambda _{\ell +1}}=\prod _{\ell =1}^{N1}\delta _{\lambda _\ell ,\lambda _{\ell +1}}\delta _{\mu _\ell ,\mu _{\ell +1}}P^{(A)}_{\lambda _1}P^{(B)}_{\mu _1}\). Products containing a commutator factor \(C_{\lambda ,\mu }\) represent a “perturbative” quantum correction to the commutative formula. Writing the product of spectral projectors as a sum over insertion of commutators, we obtain a “perturbative” expansion of \(f(A+B)\) whose first terms are given by
\(\square \)
5.2 Sum over all possible histories
From now on, we assume \(a=b=1\) for the sake of simplicity, still sticking to the case of a finitedimensional Hilbert space \({{\mathsf {H}}}\). Formula (8) allows us to construct (weakly) the spectral measure of \(A+B\) in terms of a particular limiting procedure. Let us consider, for any \(N\in {{\mathbb {N}}}\) the finite sequence of 2N observables \(O_1,\ldots ,O_{2N}\), where for \(j=1,\ldots ,N\) \(O_{2j}=A\) and \(O_{2j1}=B\). It corresponds to a sequence of alternating measurements of the couple of observables A and B. As discussed above, the statistics of these sequences of measurements is related to the complex measures \(\nu _{\phi ,\psi }^{(A,B,\dots ,A,B)}\) on \(\sigma (A)\times \dots \times \sigma (B)\) defined as
We can in this way associate with any observable \(O_n\) a map \(T(O_n)\) on \(\Omega :=(\sigma (A)\times \sigma (B))^{{\mathbb {N}}}\) as follows,
We shall henceforth set \(T(O_{2j})\equiv \xi _j\) and \(T(O_{2j1})\equiv \eta _j\), \(j\ge 1\) to shorten the notation. Formally, we have for any \(N\ge 1\) and \(f_1,\ldots , f_N, g_1, \ldots , g_N\in C_b({{\mathbb {R}}})\)
where the expectation value on the righthand side of (68) stands for the integral
Referring to a measure space \((\Omega , {\mathscr {F}}, \nu ) \), with \(\Omega = (\sigma (A)\times \sigma (B))^{{\mathbb {N}}}\), \({\mathscr {F}}\) the \(\sigma \) algebra generated by the cylinder sets (see “3”) and \(\nu \) a sigma additive measure on \({\mathscr {F}}\) with finite total variation (see Sect. 3.2), the sets \(\{\xi _n\}_{n\in {\mathbb {N}}}\) and \(\{\eta _n\}_{n \in {\mathbb {N}}}\) cannot in general be regarded as sequences of random variables (i.e., measurable functions) thereon, where \(\nu \) extends \(\nu ^{(A,B,\dots ,A,B)}_{\phi ,\psi }\). However, for any finite N the integral (69) is well defined and \(\{\xi _n\}_{n\in {\mathbb {N}}}\) and \(\{\eta _n\}_{n \in {\mathbb {N}}}\) are called pseudostochastic process. They find applications, e.g., in the mathematical definition of Feynman path integrals as well as in the construction of Feynman–Kactype formulae for PDEs that do not satisfy maximum principle [2].
In this context, the construction so far defined describes the spectral measure of \(A+B\) in terms of a particular limiting procedure. Referring to the sequence of pseudorandom variables \(\{\zeta _n\}_{n \in {\mathbb {N}}}\) defined as \(\zeta _n:=\xi _n+\eta _n\), for \(N\ge 1\) let \(S_N\) denote the map \(S_N:=\sum _{n=1}^N\zeta _n\). Then, according to formula (8), for any function \(f\in {\mathscr {F}}({{\mathbb {R}}})\) (or also \(f \in C^\infty ({{\mathbb {R}}})\) since here \(A,B \in {{\mathfrak {B}}}({{\mathsf {H}}})\) automatically because \(\dim {{\mathsf {H}}}< +\infty \)), it holds
which can be interpreted as a weak convergence of the (complex) distribution of the arithmetic mean of the first N pseudorandom variables \(\zeta _n\) to the measure \({\mathscr {B}}({{\mathbb {R}}}) \ni E \mapsto \langle \phi  P^{(A+B)}_{E}\psi \rangle \). Since we are dealing with discrete spectra, the formula above can be rephrased to
and the righthand side can be interpreted as a “sum over all possible histories.” In other words, that is an integral over the set of all possible outcomes of a sequence of consecutive measurements of the observables A and B. It is worth stressing that the same result can be obtained by means of a different construction, by considering the family of complex measures \(\nu _{\phi ,\psi }^{(B,A,\ldots ,B,A)}\) instead of \(\nu _{\phi ,\psi }^{(A,B,\ldots ,A,B)}\), describing a sequence of consecutive measurement of the observables A and B which starts with the measurement of A.
6 Summary
This work tackles the issue of connecting the spectral measure \(P^{(aA+bB)}\) of a linear combination of two observables A, B with the spectral measures \(P^{(A)},P^{(B)}\) of A and B, in the general case of a pair of noncompatible observables. This problem is relevant from the physical point of view as it helps in justifying the linear structure of the space of observables, which is assumed in the standard formulation of Quantum Theory. As a matter of fact, in Sect. 2 we establish a new formula (32), relating suitable functions \(f(aA+bB)\) of two generally noncommuting and unbounded observables A and B with their PVMs \(P^{(A)}\) and \(P^{(B)}\). That formula is the central achievement of this paper expressed by Theorem 2.5, whose proof relies essentially on Trotter formula. This constrains the class of functions f admitted by (32)—in Sect. 4 we show that the hypothesis necessary to establish our main result cannot be relaxed—however, this class of functions is nevertheless sufficiently large to allow the application of (32) to various cases of physical relevance discussed in Sect. 3. In fact, our formula has a nice interplay with the structure of Jordan algebra of observables and also with the notion of Feynman integral and the Feynman–Kac formula since, essentially, it specializes to them when A and B are suitably chosen. In addition, identity (32) has an appealing aspect from the physical viewpoint as it contains some terms which are suitable for some operational physical interpretation, as discussed in Sect. 5.
Notes
It is finally assumed that in the absence of superselection rules and gauge symmetries, the complex span of the elements in \({\mathcal{O}}_S^{(b)}\) amounts to the whole \({{\mathfrak {B}}}({{\mathsf {H}}})\); otherwise, it is a von Neumann algebra in \({{\mathsf {H}}}\).
Notice that \({\mathcal{O}}_S^{(b)}\) suffices to recover all physical information carried by \({\mathcal{O}}_S\). Indeed, for all \(A\in {\mathcal {O}}_S\) one has \(A_N := \int _{[N,N]} \lambda \hbox {d}P^{(A)}(\lambda )\in {\mathfrak {B}}({\mathsf {H}})\) (\(N\in {\mathbb {N}}\)) as well as \((A_NA)\psi \rightarrow 0\) as \(N\rightarrow +\infty \) for all \(\psi \in D(A)\). The operator \(A_N\) can be interpreted as the same observable A measured with instruments whose range is restricted to \([N,N]\).
The problem tackled in this work is a consequence of the existence of incompatible observables so that it does not arise in classical physics. Given a classical system S, for instance, described in its phase space, there is a minimal set of observables such that all remaining observables are functions of them. Therefore, measuring the first ones exactly amounts to measuring all observables of S.
From standard extension theorems of finite Borel measures as [7, Corollary 1.6.2] (whose proof is also valid for complex measures as the reader proves easily), there is only one regular complex Borel measure \(\mu \) over \({\mathbb {R}}\) determined by the values \(\mu ([\alpha , \beta ))\). If two PVMs P, Q satisfy \(\langle \phi  Q_{[\alpha ,\beta )}\psi \rangle = \mu _{\phi ,\psi }([\alpha , \beta )) =\langle \phi  P_{[\alpha ,\beta )}\psi \rangle \) for all \(\phi ,\psi \in {{\mathsf {H}}}\) and \(\alpha < \beta \) in \({\mathbb {R}}\), then it must also be \(\langle \phi  Q_{E}\psi \rangle = \mu ^{(Q)}_{\phi ,\psi }(E) =\mu ^{(P)}_{\phi ,\psi }(E) =\langle \phi  P_{E}\psi \rangle \) for every \(E\in {\mathscr {B}}({\mathbb {R}})\) and \(\phi ,\psi \in {{\mathsf {H}}}\), so that \(P=Q\).
We recall that our convention for the Fourier transform is \({\widehat{g}}(k):=(2\pi )^{1/2}\int _{{\mathbb {R}}}g(x)\hbox {e}^{ixk}\hbox {d}x\), \(g(x)=(2\pi )^{1/2}\int _{{\mathbb {R}}}{\widehat{g}}(k)\hbox {e}^{ikx}dk\) for \(g\in {\mathscr {S}}({\mathbb {R}})\)—c.f. Eq. (15).
For any partition \(\{E_j\}_j\subset \Sigma _Y\) of Y, we have that the collection of sets \(\{h^{1}(E_j)\}_j\subset \Sigma _X\) is a partition of X. Hence
$$\begin{aligned} \sum _j(h)_*\mu (E_j)=\sum _j\mu (h^{1}(E_j))\le \Vert \mu \Vert . \end{aligned}$$
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Acknowledgements
The authors are grateful to C. Fewster, R. Ghiloni and I. Khavkine for useful discussions. The authors also thank an anonymous reviewer for his/her detailed and careful suggestions to improve the text and for having pointed out further relevant bibliography.
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Appendices
Appendix A: Proof of some propositions
Proof of Lemma 2.2
(a) First of all, let us prove that there is a complex Borel measure on \({{\mathbb {R}}}^{2N}\) (with finite total variation according to Sect. 1) satisfying (21). Notice that if such a measure exists, it must be unique in view of [5, Theorem 3.3]. Let \(\{h_k\}_{k=1,..,d_n}\) be an orthonormal basis of the finitedimensional subspace \(Q_n({{\mathsf {H}}})\), where \(d_n=\text{ dim } (Q_n({{\mathsf {H}}}))\). Then,
Let us consider the unitary maps \(U^{(A)}:{{\mathsf {H}}}\rightarrow L^2({{\mathbb {N}}}\times {{\mathbb {R}}},\nu ^{(A)})\), \(U^{(B)}:{{\mathsf {H}}}\rightarrow L^2({{\mathbb {N}}}\times {{\mathbb {R}}},\nu ^{(B)})\) defined by the spectral representation of the selfadjoint operators A, B as in Theorem B.1. Setting \(h^{(A)}_j(r):=(U^{(A)}h_j)(r)\) and \(h^{(B)}_j(s):=(U^{(B)}h_j)(s)\), where \(r,s\in \Gamma := {{\mathbb {N}}}\times {{\mathbb {R}}}\) the latter equipped with the product measure when the topology on \({{\mathbb {N}}}\) is the discrete one, we have,
where we defined \(\phi ^{(A)}:=U^{(A)}\phi \), \(\psi ^{(B)}:=U^{(B)}\psi \) and
Each factor on the righthand side (like \(\overline{\phi ^{(A)}(r_1)}h^{(A)}_{k_1}(r_1)\)) is made of a product of a pair of \(L^2\) functions with the same argument (\(r_1\)); therefore, it is an element of \(L^1\) with respect to the corresponding measure \(\nu ^{(A)}\). Therefore, \(\rho ^{(n)}_{\phi ,\psi ,Q}\in L^1(({{\mathbb {N}}}\times {{\mathbb {R}}})^{2N}, (\nu ^{(A)}\otimes \nu ^{(B)})^{\otimes N})\) because it is a finite sum of \(L^1\) functions in the product measure. Hence, the set function \(\mu ^{(N,n)}_{\phi ,\psi ,Q}:{\mathscr {B}}(\Gamma ^{2N})\rightarrow {{\mathbb {C}}}\) defined as
is a \(\sigma \)additive complex measure with total variation \(\mu ^{(N,n)}_{\phi ,\psi ,Q}(\Gamma ^{2N}) \le \Vert \rho ^{(n)}_{\phi ,\psi ,Q}\Vert _{L^1}\). Let \(\Pi :\Gamma ^{2N}\rightarrow {{\mathbb {R}}}^{2N}\) be the surjective map defined by
where \(m_1,\ldots ,m_N,l_1,\ldots ,l_N\in {\mathbb {N}}\), while \(\lambda _1,\ldots ,\lambda _N,\mu _1,\ldots ,\mu _N\in {\mathbb {R}}\). Clearly \(\Pi \) is measurable because it is continuous with respect to the natural product topologies. We then define the complex measure \(\nu ^{(N,n)}_{\phi ,\psi ,Q} \) on \({\mathscr {B}}({{\mathbb {R}}}^{2N})\) extending the values \(\nu _{\phi ,\psi ,Q}^{(N,n)}(\times _{\ell =1}^nI_\ell \times J_\ell )\) as the image measure (also called pushforward measure) of \(\mu ^{(N,n)}_{\phi ,\psi ,Q}\), namely \(\nu ^{(N,n)}_{\phi ,\psi ,Q}=(\Pi )_*(\mu ^{(N,n)}_{\phi ,\psi ,Q}) := \mu ^{(N,n)}_{\phi ,\psi ,Q} \circ \Pi ^{1}\). With the said definition, if \(O \subset {{\mathbb {R}}}^{2N} {\setminus } \sigma (A) \times \cdots \times \sigma (B)\) is open, then \(\Pi ^{1}(O)\) is open and stays in the complement to the set \({{\mathbb {N}}}\times \sigma (A) \times \cdots \times {{\mathbb {N}}}\times \sigma (B)\). This set includes \(\text{ supp }((\nu ^{(A)}\otimes \nu ^{(B)})^{\otimes N})\) according to (c) Theorem B.1. Hence, \((\nu ^{(A)}\otimes \nu ^{(B)})^{\otimes N}(\Pi ^{1}(O)) =0\). Using (70) observing that \((\nu ^{(A)}\otimes \nu ^{(B)})^{\otimes N}\) is a positive measure and \(\rho ^{(n)}_{\phi ,\psi ,Q}\) is \(L^1\) with respect to that measure, we conclude that \(\mu ^{(N,n)}_{\phi ,\psi ,Q}(\Pi ^{1}(O)) =0\) which implies \(\nu ^{(N,n)}_{\phi ,\psi ,Q}(O)=0\). In other words, (22) is true.
(b) Let us define
where \(\nu _f = F^{1}(f)\) referring to (16). An elementary inductive argument establishes that
if (1) the orthogonal projectors \(Q_n\) satisfy \(Q_n \rightarrow I\) in the strong sense and (2) \(S_1, \ldots , S_N \in {{\mathfrak {B}}}({{\mathsf {H}}})\) satisfy \(\Vert S_j\Vert \le c <+\infty \) for \(j=1,\ldots ,N\). Taking advantage of this fact (noticing that \(\hbox {e}^{i s C}\) is unitary if \(s\in {{\mathbb {R}}}\) and C is selfadjoint, so that \(\Vert \hbox {e}^{i s C}\Vert =1\)), Lebesgue’s dominated convergence theorem and the Fubini theorem allow us to write
Due to (71), the limit does not depend on the chosen sequence Q as declared in the hypothesis. \(\square \)
Appendix B: Spectral representation theorem
We state and prove here a version of the spectral representation theorem for selfadjoint operators we exploited in the proof of Lemma 2.2. This is nothing but a refinement of part of some results which can be found in [25, 33].
Theorem B.1
Let \(T: D(T) \rightarrow {{\mathsf {H}}}\) a selfadjoint operator in the separable Hilbert space \({{\mathsf {H}}}\). The following facts are true.

(a)
There is a measure space \((\Gamma , \Sigma , \nu )\), where

(i)
\(\Gamma := {{\mathbb {N}}}\times {{\mathbb {R}}}\),

(ii)
\(\Sigma := {\mathscr {B}}(\Gamma )\) referred to the product topology of \({{\mathbb {N}}}\times {{\mathbb {R}}}\), equipping \({{\mathbb {N}}}\) with the discrete topology,

(iii)
\(\nu \) is a positive \(\sigma \)additive Borel measure over \(\Gamma \) which can be chosen to be finite.

(i)

(b)
There is a unitary map \(U: {{\mathsf {H}}}\rightarrow L^2(\Gamma , \Sigma , \nu )\), such that the PVM \(P^{(T)}\) of T satisfies
$$\begin{aligned} \left( U P^{(T)}_E \psi \right) (n,x) =1_E(x) (U\psi )(n,x)\quad \text{ for } \text{ every } E\in {\mathscr {B}}({{\mathbb {R}}}),\, (n,x)\in \Gamma . \end{aligned}$$(73) 
(c)
It holds \(\text{ supp }(\nu ) \subset {{\mathbb {N}}}\times \sigma (T)\).
Proof
(a) and (b). If \({{\mathsf {H}}}=\{0\}\) everything is trivial, so that we assume this is not the case. Take \(\psi _0 \in {{\mathsf {H}}}{\setminus } \{0\}\) and define the subspace \({{\mathsf {H}}}_0 := \{f(T)\psi _0 \,\, f \in L^2({{\mathbb {R}}}, \nu _{\psi _0})\}\) where henceforth \(\nu _\psi (E):= \langle \psi P^{(T)}_E\psi \rangle = \Vert P^{(T)}_E\psi \Vert ^2\). The linear map
is evidently isometric because \(\Vert f(T) \psi _0\Vert ^2 = \Vert f\Vert ^2_{L^2({{\mathbb {R}}}, \nu _{\psi _0})}\) from the elementary spectral theory [25], and surjective by construction. Furthermore, \({{\mathsf {H}}}_0\) is closed: If \({{\mathsf {H}}}\ni \psi = \lim _{n\rightarrow +\infty }f_n(T)\psi _0\), then \(\{f_n\}_{n\in {{\mathbb {N}}}}\) is Cauchy in \(L^2({{\mathbb {R}}}, \nu _{\psi _0})\) and its limit \(f\in L^2({{\mathbb {R}}}, \nu _{\psi _0})\) satisfies \(f(T)\psi _0 = \psi \). Now take \(\psi _1 \in {{\mathsf {H}}}_0^\perp \) with \(\psi _1 \ne 0\), if there is such vector, and construct an analogous isometric map
observing that \({{\mathsf {H}}}_1 \perp {{\mathsf {H}}}_0\), because \(\langle f(T)\psi _1g(T)\psi _0 \rangle = \int _{{{\mathbb {R}}}} g(\lambda ) \hbox {d}\nu _{f(T)\psi _1,\psi _0}(\lambda )\), but again from the elementary spectral theory,
We can iterate the procedure finding a class of mutually orthogonal closed subspaces \(\{{{\mathsf {H}}}_j\}_{j\in {{\mathbb {N}}}}\) and a corresponding sequence of isometric surjective maps \(V_j : L^2({{\mathbb {R}}}, \nu _{\psi _j}) \rightarrow {{\mathsf {H}}}_j\), where possibly \({{\mathsf {H}}}_{j} = \{0\}\) and \(\nu _{\psi _{j}}=0\) from some \(j_0\) on. We assume that \(\psi _j \ne 0\) for all \(j\in {{\mathbb {N}}}\) since the other case is trivial. Since \({{\mathsf {H}}}\) is separable, with a straightforward application of Zorn’s lemma, we have that the countable Hilbert orthogonal decomposition holds \({{\mathsf {H}}}= \oplus _{j=0}^{+\infty } {{\mathsf {H}}}_j\). As a consequence, \({{\mathsf {H}}}\) turns out to be isomorphic to \(\oplus _{j=0}^{+\infty } L^2({{\mathbb {R}}}, \hbox {d}\nu _{\psi _j})\) and the isomorphism is nothing but \(U' := \oplus _{j=0}^{+\infty } V_j^{1}: \oplus _{j=0}^{+\infty } {{\mathsf {H}}}_j \rightarrow \oplus _{j=0}^{+\infty }L^2({{\mathbb {R}}}, \hbox {d}\nu _{\psi _j})\,.\) Notice that taking advantage of the spectral identity \(P_E^{(T)} = 1_E(T)\), we have
where \(Q_j : {{\mathsf {H}}}\rightarrow {{\mathsf {H}}}\) is the orthogonal projector onto \({{\mathsf {H}}}_j\). At this juncture, we are free to change the normalization of the vectors \(\psi _j\) without affecting the found subspaces \({{\mathsf {H}}}_j\), requiring that \(\Vert \psi _j\Vert ^2 = 2^{j}\). With the given definitions, if \(\Gamma := {{\mathbb {N}}}\times {{\mathbb {R}}}\), \(\Sigma : = {\mathscr {B}}({{\mathbb {N}}}\times {{\mathbb {R}}})\), and \({{\mathbb {R}}}_n := \{n\}\times {{\mathbb {R}}}\), we construct the Borel measure over \(\Gamma \)
Observe that every \(E \in {\mathscr {B}}({{\mathbb {N}}}\times {{\mathbb {R}}})\) uniquely decomposes \(E=\cup _n E_n\) with \(E_n \in {\mathscr {B}}({{\mathbb {R}}}_n)\), since \({{\mathbb {R}}}_n \cap {{\mathbb {R}}}_m =\varnothing \) for \(n \ne m\). Noticing that all measures \(\nu _{\psi _n}\) are positive and \(\sigma \)additive, it is not difficult to establish that \(\nu \) is such. In particular, \(\nu \) is finite if we choose \(\Vert \psi _j\Vert ^2 = 2^{j}\), because \(\nu (\Gamma ) = \sum _{n=0}^{+\infty } 2^{n} = 2< +\infty \). Finally, it is evident that \(f \in L^2(\Gamma , \Sigma , \nu )\) if and only if \(f(n, \cdot ) \in L^2({{\mathbb {R}}}, \nu _{\psi _n})\) for all \(n \in {{\mathbb {N}}}\) and \(\sum _{n=0}^{+\infty }\Vert f(n, \cdot )\Vert ^2_{L^2({{\mathbb {R}}}, \nu _{\psi _n})} <+\infty \). In particular,
so that there is a unitary map \(U'' : \oplus _{j=0}^{+\infty } L^2({{\mathbb {R}}}, \hbox {d}\nu _{\psi _j}) \rightarrow L^2(\Gamma , \Sigma , \nu )\,,\) obviously constructed. The wanted Hilbertspace isomorphism U is therefore
With this definition, (73) is a direct rephrasing of (74).
(c) It easily arises from the standard result \(\text{ supp }(P^{(T)})= \sigma (T)\), using \(\text{ supp }(\nu _\psi ) \subset \text{ supp }(P^{(T)})\) and the disjoint decomposition of \(\Gamma \) into openclosed subsets \({{\mathbb {R}}}_n\). \(\square \)
Appendix C: Projective limit of complex measures
We state here a particular case of a general result extensively discussed in [2, 41], concerning an extension to complex measures of Kolmogorov theorem for the existence of a socalled consistent family of probability measures (see, e.g., [30, 43,44,45]). Let \({{\mathbb {N}}}\) be the index set and let us denote with \({\mathscr {F}}_{{\mathbb {N}}}\) the collection of subsets \(J\subset {{\mathbb {N}}}\) with a finite number of elements and with J the cardinality of \(J\in {\mathscr {F}}_{{\mathbb {N}}}\).
\({\mathscr {F}}_{{\mathbb {N}}}\) inherits naturally the structure of a directed set, where the partial order relation \(\le \) is defined as \(J\le K\) iff \(J\subset K\), \(J,K \in {\mathscr {F}}_{{\mathbb {N}}}\). Let us associate with any \(J\in {\mathscr {F}}_{{\mathbb {N}}}\) a measure space \({{\mathbb {R}}}^J\), naturally isomorphic to \({{\mathbb {R}}}^{J}\) and let \(\Sigma _J\) denote its Borel \(\sigma \)algebra. For any pair \(J,K \in {\mathscr {F}}_{{\mathbb {N}}}\) with \(J\le K\) let \(\pi ^K_J:{{\mathbb {R}}}^K\rightarrow {{\mathbb {R}}}^J\) be the projection map, which is continuous hence Borel measurable.
A collection \(\{\mu _J\}_{J\in {\mathscr {F}}_{{\mathbb {N}}}}\) of complex measures \(\mu _J:\Sigma _J\rightarrow {{\mathbb {C}}}\) is said to be consistent or projective if the following compatibility condition is fulfilled for any \(J,K \in {\mathscr {F}}_{{\mathbb {N}}}\), \(J\le K\):
where \((\pi ^K_J)_*\mu _K\) denotes the image (pushforward) measure of \(\mu _K\) under the action of the map \(\pi ^K_J\), namely \((\pi ^K_J)_*\mu _K (E):=\mu _K\left( (\pi ^K_J)^{1}(E)\right) \), for all \(E\in \Sigma _J\).
Let \({{\mathbb {R}}}^{{\mathbb {N}}}\) be the space of all realvalued sequences and for any \(J\in {\mathscr {F}}_{{\mathbb {N}}}\) let \(\pi _J:{{\mathbb {R}}}^{{\mathbb {N}}}\rightarrow {{\mathbb {R}}}^J\) indicate the projection map. It is simple to check that for any \(J,K \in {\mathscr {F}}_{{\mathbb {N}}}\), with \(J\le K\), the following composition property holds:
We shall consider the \(\sigma \)algebra \(\Sigma \) on \({{\mathbb {R}}}^{{\mathbb {N}}}\) generated by the cylinder sets, i.e., the subsets of the form \((\pi _J)^{1}(E)\) for some \(J\in {\mathscr {F}}_{{\mathbb {N}}}\) and \(E\in \Sigma _J\). It is simple to see that, for every complex measure \(\mu :\Sigma \rightarrow {{\mathbb {C}}}\), it is possible to define a collections \(\{\mu _J\}_{J\in {\mathscr {F}}_{{\mathbb {N}}}}\) of complex measures \(\mu _J:\Sigma _J\rightarrow {{\mathbb {C}}}\) as the pushforward of \(\mu \) under the action of the projections \(\pi _j\), i.e.,
Further, by the composition property (76), the resulting collection of measures \(\{\mu _J\}_{J\in {\mathscr {F}}_{{\mathbb {N}}}}\) is consistent, i.e., satisfies condition (75) which is indeed a necessary condition for the existence of a measure \(\mu :\Sigma \rightarrow {{\mathbb {C}}}\) generating the family \(\{\mu _J\}_{J\in {\mathscr {F}}_{{\mathbb {N}}}}\) through (77). Remarkably, in the case where the measures \(\{\mu _J\}_{J\in {\mathscr {F}}_{{\mathbb {N}}}}\) are probability measures, according to Kolmogorov existence theorem [30, 43,44,45] the consistency condition (75) is also sufficient for the existence of a probability measure \(\mu :\Sigma \rightarrow {{\mathbb {R}}}\) such that (77) holds. This result is a cornerstone of probability theory, actually providing the existence of stochastic processes. In the case where the measures \(\{\mu _J\}_{J\in {\mathscr {F}}_{{\mathbb {N}}}}\) belonging to the projective family are complex (or signed) measures, the classical Kolmogorov theorem can no longer be directly applied. Indeed, in this case, additional conditions have to be required and we refer to [41] for details. In particular, a fundamental condition is the following upper bound on the total variation of the measures belonging to the family \(\{\mu _J\}_{J\in {\mathscr {F}}_{{\mathbb {N}}}}\):
Indeed, the necessity of condition (78) can be simply proved by observing that whenever \(h:X\rightarrow Y\) is a measurable map between two measurable spaces \((X, \Sigma _X)\) and \((Y, \Sigma _Y)\) and for any complex measure \(\mu \) on \((X, \Sigma _X)\), the total variation of the pushforward measure \((h)_*\mu \) on \((Y, \Sigma _Y)\) satisfies the following inequality^{Footnote 8}
Hence, by Eq. (77), for any \(J\in {\mathscr {F}}_{{\mathbb {N}}}\) we obtain
which yields (78).
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Drago, N., Mazzucchi, S. & Moretti, V. An operational construction of the sum of two noncommuting observables in quantum theory and related constructions. Lett Math Phys 110, 3197–3242 (2020). https://doi.org/10.1007/s11005020013327
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DOI: https://doi.org/10.1007/s11005020013327
Keywords
 Noncommuting observables
 Unbounded selfadjoint operators
 Spectral measures
 Foundations of quantum theories