A local-realistic model for quantum theory

We provide a rigorous definition of local realism. We show that the universal wave function cannot be a complete description of a local reality. Finally, we construct a local-realistic model for quantum theory.


Introduction
Quantum theory has long been held to be incompatible with local realism. Local realism can be described informally, albeit incompletely, by the following principles: Principles of local realism (i) There is a real world. (ii) It can be decomposed into various parts, called systems. (iii) A system may be decomposed into subsystems. (iv) Every system is a subsystem of the global system consisting of the entire world. (v) At any given time, each system is in some state. (vi) The state of a system determines, and is determined by, the state of its subsystems. (vii) What is observable in a system is determined by the state of the system. (viii) The state of the world evolves according to some law. (ix) The evolution of the state of a system can only be influenced by the state of systems in its local neighbourhood.
The notion of local neighbourhood depends on the underlying physics. In the case of relativity theory, this would mean that no systems can influence each others if they are space-like separated. This implies that no action on a system can have an influence on another system at a speed faster than light. However, these principles are not restricted to theories in which general relativity holds.
Two reasons are usually given as to why quantum theory cannot be compatible with local realism.
The first is that quantum theory is incompatible with local hidden variable theories [1]. But those are merely a specific type of local-realistic theory. And while all local hidden variable theories are local-realistic, the converse is false. For example, the 'non-local box' introduced by Sandu Popescu and Daniel Rohrlich cannot be described by local hidden variables and yet can easily be given a local-realistic interpretation [2][3][4]. Note that the principles of local realism that we have enumerated make no reference to local hidden variables. 1 The second is that an entangled state of a composite system cannot be described in term of the states of its subsystems. This, if true, would indeed imply that quantum theory is not localrealistic. However, we shall show precisely that in quantum theory, all states of all composite systems, including entangled states, can be fully described by the states of their subsystems.
Despite these objections that are still made today, the consistency of quantum theory with local realism has already been proven by David Deutsch and Patrick Hayden [5]. They appealed to an intuitive conception of local realism that is in full agreement with the formal framework provided in this article. They also provided a local-realistic model for quantum theory. The model presented here can easily be shown to be isomorphic with theirs. Charles Alexandre Bédard provided a comparison of both models and showed their equivalence in [6,7].
But our aim here is more general. We shall present a precise formulation of the principles of local realism. From these principles, we can have precise theorems of an extremely general nature, which deal not just with quantum theory but with all possible local-realistic theories. One example is the no-signalling principle, which is valid in all local-realistic theories, and generalizes a wellknown result of quantum theory. The no-signalling principle is that no operation on a system can have an instantaneous observable effect on remote systems. That the no-signalling principle holds in all local-realistic theories is proven in a companion article, where we also show that every no-signalling theory with reversible dynamics has a local-realistic model [8]. Given that all localrealistic theories are no-signalling, this implies the following theorem: given reversible dynamics, a theory is no-signalling if and only if it has a local-realistic model.
Developing those ideas required a formalization of the concept of local realism independent of quantum theory. Developing a local-realistic model for an arbitrary no-signalling theory was obtained by abstracting away all that belongs specifically to quantum theory from the model in the current article and retaining only the most general mathematical ideas.
While the model provided in the companion article is universal, the price of universality is at a higher degree of abstraction than in the present article, which is built around the familiar density operators, vector spaces and Hilbert spaces of quantum theory. The equivalence of both models is shown in [6,7].
The local-realistic model presented in this article is valid for finite-dimensional unitary quantum theory. For the sake of brevity, in the remainder of this article, we shall often refer to finite-dimensional unitary quantum theory as quantum theory. The model of the current article can be extended to continuous-dimensional unitary quantum theory as shown in [6,7]. This paper is an extension of the doctoral work of the author, performed under the supervision of Gilles Brassard. It is intended to supersede previous work by the author on the topic [9][10][11]. In this paper, as opposed to previous work, local realism is described through explicit axioms, and greater emphasis is placed on explaining how quantum theory should satisfy these axioms. Furthermore, the local-realistic model for quantum theory and the proof that the universal wave function cannot be a complete description of local reality are presented here with full rigour and go into greater detail than the previous presentations. Nevertheless, all the key ideas were already presented by the author at a conference he gave in 2014 [10], including the main axioms of local 2. The density operator of a system does not determine the state of the system All observable properties of quantum theory can be described by the density operator formalism. A system's density operator determines to everything that is locally observable on it. However, the density operator of system A and system B do not determine the density operator of composite system AB. Yet, in a local-realistic theory, the state of composite system is determined by the state of its subsystems.
We could be tempted to jump to the conclusion that quantum theory is not local-realistic. However, this would only follow under the supposition that the state of a system is determined by its density operator.
This argument, rather than proving that quantum theory is not local-realistic gives us a hint for how to find a local-realistic model for quantum theory. Namely, by contrapositive we find that any local-realistic model of quantum theory must distinguish between the state of a system and what is locally observable in it, which, according to the principles of local-realism, is determined by the state of the system.

Local-realistic theories
Hence, our next task is to give a mathematical definition of a local-realistic theory. A local-realistic theory is defined as a mathematical theory that satisfies all the axioms we shall present. Moreover, when the local-realistic theory is quantum theory, it must also satisfy a variety of additional properties that shall be fully described later in the text. Formally, these properties should be taken as additional axioms characterizing the local-realistic theory is quantum theory.
Mathematics alone is insufficient and powerless to apprehend reality. To fully understand a physical concept such as local realism, there is by necessity an intuitive level, where the key consideration is the relation between mathematics and reality. This level by its nature cannot be discussed with the same degree of rigour. We have discussed part of the intuitive meaning of what is a local-realistic theory in the introduction of this paper. A deeper exposition of non-mathematical aspects of local realism and the relevant mathematics is given in [8].

(a) Systems
We want to define the mathematical properties of systems, where systems describe meaningful parts of the world. These systems can be combined in various ways to give rise to different systems. For example, if A is a system, there will be a system A, the complement of system A, consisting of the rest of the world. As an other example, if A and B are systems, there will be a system A B, the union of system A and B consisting of the parts of the world belonging to either of the two systems A and B.
Mathematically, systems will be represented as elements of a lattice of systems, which we define now. Definition 3.1 (Lattice of systems). A lattice of system is a six-tuple (S, , , · , S, 0), where S is a set of elements called systems, symbols , denote binary operations on the set of systems S, symbol · denotes a unary operation on the set of systems S, symbol 0 and S are distinguished elements of the set of systems S, respectively, called the empty system and the global system.
The following properties are verified for all systems A, B and C: (v) Complementation: Formally, a lattice of system is simply a Boolean lattice. However, we believe that an evocative terminology helps to build proper intuition, thus the properties of Boolean lattices are better described using the terminology of physical systems, rather than the general but flavourless language of Boolean lattices.
Conceptually, the global system could represent as much as the entire universe, or a much smaller system. Though our goal is ultimately to be able to represent as much as possible, we might want to describe in a local-realistic way smaller systems like a quantum computer or several qubits.
Given the definition of a lattice of systems, we can state the first axiom.
We now introduce some terminology on systems. There is a natural partial order ' ' among systems defined by

Definition 3.3 (Proper subsystem).
A system B is a proper subsystem of a system A if B is a subsystem of A and B is distinct from the empty system 0 and system A.
It can be verified that A∈A A is a system. It can further be verified that for all finite sets of systems A and B We could have defined the finite intersection in the same way, but shall not need to do so for the purpose of this article.
The following theorem is a well-known theorem of finite Boolean lattices, expressed in the terminology of systems. We shall refer to A as the atomic decomposition of B. We shall soon discuss properties of systems in quantum theory, and for that, we will need to work with the tensor product of Hilbert spaces. To fix some notation, we first define what is meant by a tensor product. Definition 3.10 (Tensor Product). Let F be a field, let V 1 , V 2 , V 3 be vector spaces over the field F and let ⊗ : V 1 × V 2 → V 3 be a bilinear operation. We say that (V 3 , ⊗) is a tensor product of V 1 and V 2 if for all vector spaces W over the field F, and all bilinear functions f : V 1 × V 2 → W, there exists a unique linear application g : V 3 → W such that for all vectors v 1 of V 1 and all vector v 2 of V 2 , the following holds: If (V 3 , ⊗) is a tensor product of V 1 and V 2 , we write V 3 = V 1 ⊗ V 2 and we also refer to operation ⊗ as a tensor product.
With slight modifications, this is the category-theoretic definition of a tensor product.

(i) Systems in finite-dimensional unitary quantum theory
When the local-realistic theory is finite unitary quantum theory, its associated lattice of systems is finite, and associated with each system A is a finite-dimensional complex Hilbert space denoted H A . Furthermore, if system A is distinct from the empty system, its associated Hilbert space H A is of a dimension larger than one. This implies that given a non-empty system A, the Hilbert space H A associated with system A always contains at least two orthonormal vectors. Thus, a non-empty system A contains at least a qubit of information. Also, associated with every pair of disjoint system A and B is a tensor product ⊗ (A,B) such that Moreover, the family of tensor products satisfies the two following properties for any arbitrary mutually disjoint system A, B and C, and any arbitrary vectors |u A , |v B , |w C belonging, respectively, to the Hilbert spaces of systems A, B and C These properties are consistent with the fact that since system AB is equal to system BA, their underlying Hilbert spaces are identical, and also that since system (AB)C is identical with system A(BC) their underlying Hilbert spaces are also identical. When there is no ambiguity, we shall drop the subscripts and write ⊗ to denote all tensor products. For example, the two lines above shall be written as Since the tensor product behaves associatively, as an abuse of notation we shall omit the unnecessary parentheses and write |u A ⊗ |v B ⊗ |w C to denote the tensor product of |u A , |v B and |w C . Also, the associated Hilbert space of the empty system 0 is equal to the field of complex number C. Furthermore, for an arbitrary system A, the tensor products ⊗ (0,A) and ⊗ (A,0) verify and also for any complex number c and vector |v A ,

(b) States
We now turn our attention to the states of systems. As we discussed previously in §2, we need to distinguish between what can be locally observable in a system and its complete description. This leads us to the distinction between two kinds of states for a system.
The noumenal state of a system is its complete local description. The phenomenal state of a system is a complete description of what is locally observable in that system.
The 'noumenal/phenomenal' terminology is inspired by Kant's; however, our usage should neither be taken as an endorsement of Kantian metaphysics nor as a claim that our usage conforms to his [12,13].
This leads us to corresponding axioms . Associated to a system A is noumenal state space, Noumenal-Space A , which is a non-empty set of noumenal states.
Particular noumenal states of A will be denoted N A , N A i , N A 1 , etc. Intuitively, the noumenal state space of a system consists of all possible noumenal states that it could theoretically be in. Axiom 3.3 (Phenomenal state space). Associated with a system A is a phenomenal state space, Phenomenal-Space A , which is a non-empty set of phenomenal states.
Particular phenomenal states of A will be denoted ρ A , ρ A i , ρ A 1 , etc. Intuitively, the phenomenal state space of a system consist of all possible phenomenal states that it could theoretically be in.

(i) States in quantum theory
In quantum theory, given a Hilbert space H, we will denote the set of density operators on the Hilbert space H as Density-Operator H = {ρ : ρ is a density operator on H}.
In quantum theory, the phenomenal state space of a system A, with associated Hilbert space However, the density operator formalism of quantum theory does not supply noumenal states. Therefore, noumenal states will need to be given later in order to provide quantum theory with a local-realistic model.
(ii) Pure state quantum theory A variant of quantum theory, which we shall call pure state quantum theory, is like quantum theory subject to the restriction that the states of the global system are pure. Formally, we shall say that a density operator ρ on Hilbert space H is a pure density operator on H if there exists a unit vector |τ in H such that ρ = |τ τ | .
Thus in pure state quantum theory, the phenomenal space for the global system S is instead Pure-Phenomenal-Space S def = {ρ S : ρ S is a pure density operator on H S }.
For every other system A, the phenomenal space of that system shall consist exclusively of density operators on H A that are partial traces of pure density operators belonging to H S . Formally, Everything else remains unchanged.

(c) Operations and actions
We now want to describe how states can evolve in a local-realistic theory. The evolution of a system happens through operations that can be applied to the system. The precise operation that is applied might depend on various factors including time, the dynamical laws of physics and the environment external to the 'global' system, which might be empty if the global system is the whole universe.
The next definition characterizes the mathematical properties of a set of operations that can be performed on a system and how these operations may be combined into new operations.  where Operations is a set whose elements are called operations. The set of operations comes with a binary operator denoted '•', called the composition, and I is an operation called the identity operation. A monoid of operations satisfies the following properties: When there is no ambiguity, we shall omit the composition operator and write UV instead of U • V. Now:

Axiom 3.4 (Operations on a system). Associated with a system A is a monoid of operations, (Operations
Particular operations on system A are denoted U A , V A , etc. Also, I A denotes the identity operation on system A. When there is no ambiguity, we drop the superscript and write simply U, V and I.
Intuitively, the operations associated with a system are the operations that can be performed on the system, and if U and V are operations on a system, the operation U • V can be implemented by first doing V, followed by doing U.

(i) Operations in quantum theory
In quantum theory, the set of operations on system A with associated Hilbert Space H A is The composition of operations U and V is simply their composition as linear operators. Finally, I A is the identity operator on H A .
An operation can act on a state to produce a new state, as follows: Definition 3.12 (Operation action). Let (Operations, •, I) be a monoid of operations and S be a set. An operation action of the monoid of operation on set S is a binary operator : Operations × S → S that satisfies, for all operations U and V and for all elements s of the set S, The next two axioms use the above definition to express the fact that an operation done on a system changes its underlying noumenal and phenomenal state.

Axiom 3.5 (Noumenal action)
. Associated with a system A, is a noumenal action denoted ' A ', which is an operation action of the monoid of operations of the system on the set of noumenal states of the system.
When there is no ambiguity, we drop the superscript of the noumenal action. For example, we write U N A instead of U A N A . Intuitively, if system A was in noumenal state N A , and an operation U is done on it, its new noumenal state is U N A . Axiom 3.6 (Phenomenal action). Associated to a system A is a phenomenal action '· A ', which is an operation action of the monoid of operations of the system on the set of phenomenal states of the system. When there is no ambiguity, we drop the superscript of the phenomenal action. For example, Intuitively, if a system A was in phenomenal state ρ A , and an operation U is done on system A, its new phenomenal state is U · ρ A .

(ii) Phenomenal action in quantum theory
In quantum theory, we do not have yet noumenal states, and hence no noumenal action either, but the phenomenal action of a unitary operation U on a state ρ is defined by the theory as where UρU † is obtained through the usual composition of linear operators U, ρ and U † .

(d) Noumenal-phenomenal homomorphism
In a local-realistic theory, what is observable locally in a system is determined by the complete description of that system, in other words, the noumenal state of a system determines its phenomenal state. If the noumenal state of a system evolves according to an operation, its corresponding phenomenal state must evolve according to the same operation. Mathematically, the phenomenal state of a system will be determined by its underlying noumenal state, through a structure-preserving surjective map: a noumenal-phenomenal epimorphism. But first Definition 3.13 (Noumenal-phenomenal homomorphism). Let A be a system and let φ be a mapping whose domain is the noumenal state space of A and whose range is the phenomenal state space of A. We say that φ is a noumenal-phenomenal homomorphism on system A if, for any operation U of system A and any noumenal state N of A, When no ambiguity can arise, we omit the noumenal action. For example, the equation above becomes However, we never omit writing the phenomenal operation action because there is a possible ambiguity in quantum theory at the phenomenal level: we need to distinguish between the action of unitary operation U on phenomenal state ρ, and the composition of linear operator U with linear operator ρ.

Definition 3.14 (Noumenal-phenomenal epimorphism).
A surjective noumenal-phenomenal homomorphism on system A is called a noumenal-phenomenal epimorphism on system A.

Axiom 3.7 (Noumenal-phenomenal epimorphism). Associated with each system
When there is no ambiguity, we write ϕ instead of ϕ A . Intuitively, if a system A is in noumenal state N A , it has a corresponding phenomenal state ρ A = ϕ(N A ). Furthermore, if an operation U is done on system A, its new noumenal state is UN A , and its corresponding new phenomenal state is U · ρ A . Lastly, every phenomenal state on a system arises from at least one noumenal state, since what is observable has an underlying reality.
In unitary quantum theory, we have not yet provided noumenal states, or therefore any noumenal-phenomenal epimorphism. One task ahead is to supply it.

(e) Partial traces
The next axioms express the fact that the noumenal state of a system determines the noumenal state of any of its subsystems.  Associated with all pairs of disjoint systems A and B is a function denoted tr AB B , which is called the noumenal partial trace of system B from system AB. Partial trace tr AB B is a surjective function from the noumenal space of system AB to the noumenal space of system A.
Furthermore, for any noumenal state N ABC belonging to a composite system ABC, then the following relation must hold between partial traces: When there is no ambiguity, we shall omit the superscript and we shall refer to tr B as the noumenal partial trace of system B, regardless of the supersystem from which it is obtained by tracing. For example, the previous equation will simply be written as Intuitively, if a composite system AB is in noumenal state N AB , the noumenal state of system A will be N A = tr B (N AB ).
The next axiom expresses the fact that the phenomenal state of a system determines the phenomenal state of any of its subsystems.

Axiom 3.9 (Phenomenal partial trace). Associated with all pairs of disjoint systems A and B
is a function called the phenomenal partial trace of system B from system AB. These phenomenal partial traces follow the same requirements as noumenal partial traces, as stated in axiom 3.8, mutatis mutandis. As an abuse of notation, we also denote the phenomenal partial trace of system B from system AB by tr AB A , since no ambiguity will be possible with the corresponding noumenal partial trace tr AB A .
Finally, when there is no ambiguity, we shall omit the superscript and we shall refer to tr B as the phenomenal partial trace of system B, regardless of the supersystem from which it is obtained by tracing.
Intuitively, if a composite system AB is in phenomenal state ρ AB , the phenomenal state of system A will be ρ A = tr B (ρ AB ).

(i) Partial traces in quantum theory
In quantum theory, the phenomenal partial traces are the familiar partial traces of linear algebra. However, we do not have yet noumenal partial traces.
The next axiom expresses the consistency between the noumenal and phenomenal partial traces.

Axiom 3.10 (Relation between noumenal and phenomenal partial traces).
For all composite systems AB, and all noumenal states N AB , the noumenal and phenomenal partial traces of the system B are related by the following commuting relation: Here, the symbol ϕ stands for ϕ AB on the left side of the equation, but for ϕ A on the right side. Also, the symbol tr B stands for the phenomenal partial trace on the left side of the equation, but for the noumenal partial trace on the right side.

(f) Noumenal product
We shall need the following definition to express the next axiom.  The next axiom expresses the requirement that the state of a system is determined by the state of its subsystems.

Axiom 3.11 (Noumenal product).
Associated with all disjoint systems A and B is an operation, the noumenal product, denoted ' ', 2 such that for all noumenal states N AB , the following equation holds: There is no corresponding axiom for a phenomenal product, and this is the most profound distinction between the noumenal and phenomenal level.
Unitary quantum theory does not yet provide us with a noumenal product, so we shall need to provide it.
The following theorems give important properties of the noumenal product.

Theorem 3.3 (Unique decomposition). Let A and B be disjoint systems, then
Proof. We prove N A 1 = N A 2 ; the other statement is similar. We apply theorem 3.2 and get

(g) Product of operations
Intuitively, the next axiom tells us what happens to the noumenal state of composite system AB, if an operation U is performed on system A and an operation V is performed simultaneously on system B.

Axiom 3.12 (Product of operations).
Associated with all disjoint systems A and B is a product of operations, which we denote '×'. 3 Given operations U on system A and V on system B, U × V, the product of U and V is an operation on system AB that satisfies the following relation for any noumenal state

(i) Product of operation in quantum theory
In unitary quantum theory, the product of operations is the usual tensor product ⊗. 4 Of course, we will need to verify that the tensor product satisfies axiom 3.12. This concludes our statement of the axioms that characterize a local-realistic theory.

(h) No action at a distance versus no-signalling
We now state two theorems that hold for arbitrary local-realistic theories. This will help us clarify the difference between two important facets of locality, which we shall need when we analyse Everett's conception of quantum theory and contrast it with the approach in the present article.
In a local-realistic theory, no action on a system can have any effect whatsoever on any other non-interacting system. This is formalized as follows: Theorem 3.5 (No action at a distance). Let N AB be a noumenal state of composite system AB. For all operations U on system A and V on system B, Intuitively, the no-action at a distance theorem states that no operation V performed on system B can have a noumenal effect on a remote system A.
This theorem implies another important, albeit obvious, consequence of a theory being localrealistic. If no action on a system can have any effect on any other non-interacting system, then no action on a system can have any observable effect on any other non-interacting system. This is formalized in the following theorem, valid in all local-realistic theories, which is a generalization of a well-known theorem of quantum theory. Theorem 3.6 (No-signalling principle). Let ρ AB be a phenomenal state of system AB. For all operations U on system A and V on system B, Proof. See [8].
Intuitively, the no-signalling principle means that no operation V applied on system B can have a phenomenal (i.e. observable) effect on a remote system A.
The no-signalling principle is the phenomenal counterpart of the no-action at a distance theorem. It can be satisfied in a purely phenomenal theory, one without any mention of noumenal states, in contrast to the no-action at distance theorem, which refers to noumenal states. 5 4. Interlude: the universal wave function cannot be a complete description of a local reality In his doctoral dissertation Hugh Everett III introduced a fascinating idea, the theory of the universal wave function, which led to the development of unitary quantum theory [14,15]. -At all times, the state of universe is described, up to irrelevant phase factor, by a unit vector in the Hilbert space of the universe, called the universal wave function of the universe. -All systems, including observers, are quantum systems, there are no classical systems. -All interactions between systems are described by unitary operations. This implies that what was previously described as a measurement of a quantum system by an observer is reduced to an ordinary unitary operation involving the observing system, the observed system and the environment. Also, any interaction between what was previously described as two classical systems, for example the sending of classical information, is also described by a unitary operation. -The universal wave function of the universe evolves according to a global unitary operation.
Importantly, the goal of Everett was not to give a local-realistic explanation for quantum theory, but rather to remove the arbitrary distinction between classical systems and quantum systems and therefore to analyse all interactions between systems as quantum interactions. Nevertheless, he believed that his approach could resolve the various paradoxes that plagued quantum theory, including the Einstein-Podolsky-Rosen paradox [16]. As he wrote in his thesis [14] It is therefore seen that one observer's observation upon one system of a correlated, but noninteracting pair of systems, has no effect on the remote system, in the sense that the outcome or expected outcome of any experiments by another observer on the remote system are not affected. Paradoxes like that of Einstein-Rosen-Podolsky which are concerned with such correlated, non-interacting, systems are thus easily understood in the present scheme.
Here, Everett is expressing in the language of probabilities the idea that the theory of the universal wave function obeys the no-signalling principle, i.e. theorem 3.6. 6 In his thesis, Everett described the states of subsystems as mixtures of pure states. This description determines the density operator of a given subsystem. Nevertheless, he recognized that the mixture of pure state description was insufficient to give a fully local description of entangled subsystems. As he wrote in his thesis [14] However, this representation by a mixture must be regarded as only a mathematical artifice which, although useful in many cases, is an incomplete description because it ignores phase relations between the separate elements which actually exist, and which become important in any interactions which involve more than just a subsystem.
Thus Everett was well aware of the problem of locality in quantum theory, and knew that he did not give a complete local description of the states of subsystems, merely a useful description of what is locally observable in a subsystem. Describing the state of subsystems as mixture of pure states is silent about the most important facet of locality, namely the possibility to retrieve the complete state of a system from the states of its subsystems, which is expressed mathematically by the existence of a noumenal product. This also implies that the no-action at a distance principle, theorem 3.5, cannot be addressed with this description.
But what about the universal wave function itself, is it too a 'mathematical artifice', insufficient to describe a truly local-realistic theory, but nevertheless a useful description? Or could we take the wave function as a complete local-realistic description of the state of the universe, and find a truly local description of the states of subsystems?
Thus our purpose is to answer the following question: Can the universal wave function be a complete description of a local reality? Or, to phrase it according to our terminology, is there a local-realistic model of quantum theory where the noumenal state of the universe can be described by the universal wave function proposed by Everett? Certainly, the universal wave function determines everything that is observable in the universe. Therefore, at the very least, it determines the phenomenal state of the universe.
We now prove that the universal wave function cannot be a local-realistic description of the noumenal state of the universe. For this purpose, suppose we are given a local-realistic model of pure state quantum theory. Thus for each system A, we are given (ii) A noumenal space, which consists of a set of noumenal states.
(iii) A set of phenomenal states, namely Pure-Phenomenal-Space A , whose elements are density operators on system A. (ix) A noumenal-phenomenal epimorphism.
For each disjoint system A and B, we are also given a noumenal product and a product of operation, which is the usual tensor product.
We now make the following three suppositions, which correspond to the idea that the universal wave function is a description of the noumenal state of the universe. (iii) The noumenal-phenomenal epimorphism ϕ S on the global system S is the function that sends a unit vector |τ to its corresponding density operator |τ τ |.
The reader can easily verify that we have indeed defined a noumenal action on the global system and that ϕ S is indeed a noumenal-phenomenal epimorphism on the global system.
Lastly, we need to make the additional hypothesis that the theory contains at least one nontrivial system. Recall that a system A is non-trivial if it is neither the empty system nor the global system S. This hypothesis is made so that the theory contains at least two disjoint systems, each of which contain at least one qubit. Using this hypothesis, we take an arbitrary non-trivial system A. System A being non-trivial implies that its complement B is also non-trivial. Since neither A nor B is the empty system, their associated Hilbert spaces H A and H B are of a dimension greater than one. Thus the Hilbert space of system A contains at least two orthonormal states, |0 A and |1 A , and the Hilbert space of its complement, system B, contains at least two orthonormal states, |0 B and |1 B .
Our argument will make use of the following Bell States: and In a local-realistic theory, all noumenal states can be written as a product state, in particular the Bell State, |Ψ + AB can be written as a product state However, by using axiom 3.12 again, we obtain Since |Φ + AB = |Ψ + AB , we have reached a contradiction! It follows that the universal wave function cannot be the complete description of a local universe. It merely determines what can be observed, namely the phenomenal state of the universe. Seen this way, if we believe in a local universe, the answer to the question posed in the title of the EPR 1935 paper is: 'NO, (the-then-standard) quantum-mechanical description of physical reality CANNOT be considered complete'. In other words, the universal wave function is but a shadow of the real world, which is fully described only at its noumenal level! In electronic supplementary material, A, we go further and show that in an arbitrary localrealistic model of quantum theory (containing at least one non-trivial system), for any non-empty system, the noumenal-phenomenal epimorphism associated with that system is not injective. Thus the noumenal space of a (non-empty) system must be distinct from (and larger than) its corresponding phenomenal space. Therefore, the distinction between the noumenal world and phenomenal world is mathematically necessary. Under the hypothesis that if a mathematical quantity is necessary to describe reality, that quantity corresponds to something that is real, and that quantum theory is local-realistic and describes reality, then this larger noumenal world is real and cannot be described by its wave function alone.

Construction of a local-realistic model for quantum theory
We now construct a local-realistic model for quantum theory. Specifically, recall that we are given a finite lattice of systems. For each system of those systems, we are given (i) A Hilbert space, (ii) A phenomenal state space consisting of density operators on the Hilbert space, (iii) A monoid of operations consisting of the unitary operations on the Hilbert space of the system, (iv) A phenomenal action of the operations on the phenomenal state space, which is the usual application of a unitary operation on a density operator, (v) A partial phenomenal trace, which corresponds to the usual partial trace of a density operator.
Our goal is to construct for each system For each pair of disjoint systems, we also need a noumenal product. We also need to verify that all axioms of a local-realistic theory are satisfied. The proof will be done in two steps, first we will construct a model for pure state quantum theory, then we shall use the objects created in that construction to construct a model for quantum theory.
Our first goal is to associate with each system A a specific orthonormal basis B A of its Hilbert space H A . For that purpose, we introduce some concepts related to orthonormal bases and their product.

(i) Product of orthonormal bases of Hilbert spaces
Let B 1 be an orthonormal basis of Hilbert space H 1 and B 2 be an orthonormal basis of Hilbert space H 2 . We define the tensor product of B 1 and B 2 to be It is well known that B 1 ⊗ B 2 is an orthonormal basis of Hilbert space H 1 ⊗ H 2 .
We shall now extend the notion of a product of two orthonormal bases to a finite product of orthonormal bases. Let A be a set of mutually disjoint systems, and for each system A of A, let B A be an orthonormal basis associated with system A. Recall that the Hilbert space associated with the empty system 0 is equal to the field of complex numbers C and that the singleton set {1} is an orthonormal basis of C. We define recursively A∈A B A in the following way: It can be verified that A∈A B A is an orthornomal basis of the Hilbert space associated with system A∈A A.
It can also be verified that A∈{A} B A = B A . Furthermore, if A, A are finite sets of disjoint systems such that A and A are disjoint sets, i.e. A ∩ A = ∅, it can verified that

Theorem 5.1. There exists a family (B A ) A∈S indexed by the set of all systems S, such that for every system A, B A is an orthonormal basis of the Hilbert space associated with A. Furthermore, for all composite system AB, the following relation holds between the basis of composite system AB and the bases of subsystems A and B
Proof. For each atomic system A , we associate an arbitrary orthonormal basis B A . If A is any non-atomic system with atomic decomposition A, we associate it with the orthonormal basis B A = A ∈A B A . Note that trivially, when a system A is atomic, its atomic decomposition is {A} and Thus, we have obtained a family of orthonormal bases (B A ) A∈S such that for all systems A with atomic decomposition A, the following relation is satisfied: We now verify that the family of orthonormal bases (B A ) A∈S has the property that for every composite system AB, We now fix an arbitrary family of bases (B A ) A∈S satisfying the hypotheses of theorem 5.1. We shall refer to the basis B A of system A, as the canonical basis of system A.
We shall use this fixed family of canonical bases to construct noumenal states. To that end we introduce some definitions and concepts.
Given a vector space V, we shall denote by L(V) the set of linear maps from V to itself. More formally, For the purpose of this article, all indexed orthonormal bases will be implicitly assumed to be faithfully indexed. This condition will be necessary for sums over indices. Importantly, if two operator matrices share the same entries (with respect to the same indexing for B A ), it follows that they are equal.
Note that while the entries of the operator matrix M A are implicitly dependent on the indexing for the basis B A , the operator matrix itself is not.

Definition 5.4 (Evolution Matrix).
Let A be a system with associated Hilbert space H A , let W be a unitary operation on the global system S, and let B A = {|i } i∈I be an orthonormal basis of H A . The evolution matrix [W ] A B A of operation W in the basis B A of system A is an operator matrix in basis B A whose entry ij is the operator

Definition 5.5 (Evolution space).
Let A be a system. Let B be an orthonormal basis of the Hilbert space H A associated with system A. We define the space of evolution matrices for system A, in basis B as

Evolution-Space
We give additional properties and theorems that relate evolution spaces in different bases in electronic supplementary material, B.

(ii) Noumenal states
We are now ready to define the noumenal space of system A in the following way: Let A be a system and let B A be its canonical basis,

Noumenal-Space
When there is no ambiguity, we shall omit the subscript denoting the basis of an evolution matrix

when [W]
A is a noumenal state of system A, the omitted basis is always the canonical basis of system A.
Thus an arbitrary noumenal state N A of system A is an evolution matrix in canonical basis B A = {|i } i∈I for which there exists a unitary operation W belonging to the global system S such that N A = [W] A . Therefore, noumenal state N A is an operator matrix, and we shall denote its ij entry by N A ij .

Theorem 5.2 (Fundamental property of noumenal states). For every system A, every unitary operation V on its complement, and every unitary operation W on the global system
Proof. Recall that if two matrices share the same entries then they are equal.
Definition 5.6 (Action of a unitary operator on a noumenal state). Let A be a system, let B A = {|i } i∈I be the canonical basis of the associated Hilbert space H A . Let U be a unitary operation on system A. Let N A be a noumenal state of A. We define the action of U on N A to be the operator matrix U A N A in basis B A whose entry ij is defined as where U ik is the entry ik of unitary operator U in basis B A and U † lj is the lj entry of unitary operator U † in basis B A .
Note that U ik , U † lj are scalars while N A kl is a linear operator. Thus the product U ik N A kl U † lk is obtained through the ordinary multiplication of a linear operator by scalars.
When there is no ambiguity we may omit the superscript of the action symbol and write simply U N A instead of U A N A . Further, when there is no ambiguity, we may also omit writing the symbol altogether, for example writing UN A instead of U N A . It remains to prove that we defined a proper action at the noumenal level and thus that axiom 3.5 is satisfied. This follows from the next three theorems. Proof.

Theorem 5.3 (Fundamental property of the noumenal action). For all systems A, for all unitary operations on A, and all unitary operations W on the global system S, the following holds:
The theorem 5.3 implies that the action of a unitary operation on a noumenal state is indeed a noumenal state. It follows that for all systems A, we are justified in writing that

Theorem 5.4. For every system A and all operations U and V on system A, and for every unitary operation W on the global system S,
Proof.

Theorem 5.5. For all systems A, and every unitary operation W on the global system S,
Proof.
There is an important lesson hidden in the proof of the three last theorems. Note that we have defined an action and verified that it satisfies the fundamental property of the noumenal action, namely theorem 5.3. This theorem has been proven by verifying that the entries of both operator matrix U[W] A and [(U ⊗ I A )W] A are equal. A proof that examines only entries of matrices belongs exclusively to linear algebra. However, we have then used theorem 5.3 to prove theorems 5.4 and 5.5, without reference to entries of matrices. Such a proof can be more easily generalized beyond linear algebra. Many of the proofs that follow are built on similar ideas, where generalization is kept in mind. We will prove that a fundamental property is satisfied by certain linear operators by showing an equality by entries, and then use this fundamental property to prove theorems without any appeal to properties of the entries of the matrices. There is another key to generalization. We could have alternatively taken the fundamental property of noumenal actions to be the definition of the noumenal action. This is what was done in [8]. Doing this completely eliminates the need to work with entries of matrices.

Definition 5.7 (Noumenal partial trace).
Let AB be a composite system, let B A = {|i } i∈I be the canonical basis of system A, and B B = {|k } k∈K be the canonical basis of system B. Recall that the canonical basis of system AB is Let N AB be a noumenal state of system AB. Define tr AB B (N AB ), the noumenal partial trace of N AB with respect to system B, as the operator matrix in basis B A whose entry ij is defined as As usual, when there is no ambiguity, we omit the superscript and write tr B instead of tr AB B . It remains to verify that what we have defined satisfies the axiom 3.8 for noumenal partial traces. This is a consequence of the next three theorems.
Theorem 5.6 (Fundamental property of the noumenal partial trace). Let AB be a composite system, let [W] AB be an arbitrary noumenal state of system AB, Proof. Recall that two matrices of operators are the same if they share the same entries. Let C be the complement of composite system AB; thus ABC = S, where S is the global system.
Theorem 5.6 implies that a noumenal state of system AB is sent to a noumenal state of system A by noumenal partial trace tr AB B . Thus we are justified in writing

Definition 5.8 (Noumenal product).
Let AB be a composite system, let B A = {|i } i∈I , and B B = {|k } k∈K be the canonical bases of systems A and B, respectively. Let N A and N B be mutually compatible noumenal states of systems A and B, respectively. We define N A N B , the noumenal product of N A and N B , to be the operator matrix in canonical basis Note that N A ij N B kl denotes the ordinary composition of operators N A ij and N B kl , both of which are linear operators belonging to L(H S ) . Theorem 5.9 (Fundamental property of the noumenal product). For any composite system AB, for all unitary operation W on global system S, Proof. Let C be the complement of composite system AB, so ABC is the global system S.
The next theorem proves that the noumenal product satisfies axiom 3.11. Proof.
With the next theorem, we prove that the product of operations satisfies axiom 3.12.

Theorem 5.11. Let AB be a composite system, let U and V be unitary operations on A and B, respectively, and let [W] AB = [W] A
[W] B be an arbitrary noumenal state of system AB, then the following equation is satisfied: Proof. Let C be the complement of composite system AB, thus ABC = S, where S is the global system. A to be the density operator φ A ρ (N A ), for which the ij entry of the corresponding density matrix in canonical basis B A satisfies We now verify that in quantum theory, for each ρ in the phenomenal space of the global system S, function φ A ρ is indeed a noumenal-phenomenal homomorphism on system A. This follows from the two next theorems. Theorem 5.12 (Fundamental property of the noumenal-phenomenal homomorphism). For every system A, every phenomenal state ρ of the global system S and every unitary operation W of the global system, Proof.
Theorem 5.12 shows that for all systems A, the application of φ A ρ on an arbitrary noumenal state [W] A indeed gives a density operator on system A, namely the partial trace applied to the complement of system A on the density operator W · ρ = WρW † . Therefore, we may write Theorem 5.13. For every system A and for every ρ in the phenomenal space of the global system, the function φ A ρ is a noumenal-phenomenal homomorphism and satisfies

for any noumenal state [W] A and unitary operation U on A.
Proof.
When there is no ambiguity, we shall omit writing the superscript indicating the system on which a noumenal-phenomenal homorphism act. Thus we shall write φ ρ instead of φ A ρ . The next theorem shows that for each ρ in the phenomenal space of the global system S, the noumenal-phenomenal homomorphism φ ρ satisfies axiom 3.10 on the relation between noumenal and phenomenal partial traces. Proof. Let C = AB, i.e. S = ABC, We now prove that for any pure density operator ρ on the Hilbert space H S of the global system S, function φ A ρ is a noumenal-phenomenal epimorphism in pure state quantum theory. This is the purpose of the following two theorems. Proof. Since ρ is a pure density operator of the global system S, it follows that W · ρ is also a pure density operator of the global system, and thus that tr , the theorem follows.
By theorem 5.15, when ρ is a pure density operator it follows that either: depending on whether we work in pure state quantum theory or in quantum theory.
Thus, we may fix an arbitrary pure density operator ρ in the phenomenal space of the global system S and associate with each system A the noumenal-phenomenal epimorphism φ A ρ . This completes the construction of a local realistic model for pure state quantum theory. Note that for any pure density operator ρ on global system S, φ S ρ is a noumenal-phenomenal epimorphism in pure state quantum theory, but it is not one in general in quantum theory, because is not surjective in any theory containing mixed states. There will be mixed states in quantum theory whenever the global system S is distinct from the empty system. Now that we have a model for pure state quantum theory, we will create a model for quantum theory. We shall achieve this by the redefinition of the noumenal states, the noumenal actions, the noumenal partial traces, the noumenal products and the construction of the noumenalphenomenal epimorphisms. These new objects will be constructed by using the objects previously constructed for the model in pure state quantum theory.
Let A be a system, we define the new noumenal state of system A to be

New-Noumenal-Space
Thus an arbitrary new noumenal state of system A will be of the form ([W] A , ρ) for some unitary operation W on the global system, and some density operator ρ of the global system. The new noumenal product is a partial function, where (N A , ρ 1 ) (N B , ρ 2 ) is defined only whenever ρ 1 = ρ 2 and that A and B are disjoint systems and that N A N B is already defined according to the original noumenal product . The new noumenal-phenomenal epimorphism ϕ A on system A is defined as follows: It is easy to verify that the new objects constructed, including the noumenal-phenomenal epimorphisms, satisfy all the axioms of a local-realistic theory. The verification is tedious but straightforward. The next two theorems are given as way of examples of how the axioms are verified. First, axiom 3.11. We now prove that the axiom 3.10 concerning the relation between noumenal and phenomenal partial traces is satisfied. tr B (ϕ AB (N AB , ρ)) = ϕ A (tr B (N AB , ρ)).
Note that on the left, we have the phenomenal partial trace, which is unchanged, while on the right, we have the new noumenal partial trace.
Note that we used theorem 5.14.
Furthermore, for each system, ϕ A is indeed a noumenal-phenomenal epimorphism, which was the object of the exercise of defining 'new' objects. To prove this, it suffices to show that for each system A, ϕ A is a noumenal-phenomenal homomorphism (which is obvious) and that ϕ A is surjective, as follows: Theorem 5.19. Let A be a system, Proof. Let ρ A be an arbitrary density operator of system A. We show that there exists (N A , ρ) in New-Noumenal-Space A such that ϕ A (N A , ρ) = ρ A . Let ρ A be any density operator on system A, thus ρ A ⊗ ρ A is a density operator on the global system S. Let ρ = ρ A ⊗ ρ A . Recall that I S is the identity operation on global system S.
The existence of the required noumenal-phenomenal epimorphism is established for each system, which concludes our construction of a local-realistic model for quantum theory.
For an explanation of how the model works in practice, see [7].

Conclusion
The goal of this article was to give a precise definition of local realism and to show that quantum theory is local-realistic by proving that it has a local-realistic model. The key idea allowing this was to distinguish between what can be observed locally in a system and the complete local description of the system. Prima facie, one might have hoped that, as in classical physics, the noumenal world-as-itis would be equivalent to the phenomenal world as it could be observed. But in quantum theory, there exist entangled systems, in states that defy any local-realistic explanation equating observable with real. This forces us to distinguish noumenal from phenomenal.
Given a precise definition of local-realism and a rigorous local-realistic model for quantum theory, we might wonder why such a model exists. The precise answer is in ref. [8]. It is that any theory that conforms to the no-signalling principle has a local-realistic model. In other words, a theory forbids action at a distance if and only if it forbids observable action at a distance. That, in turn, leads to perhaps the deepest question: 'Is quantum theory local-realistic?' In a discussion with the author, David Deutsch remarked Locality is not a symmetric property. If a theory has no local-realistic model, it is obviously non-local. However, if a theory has a local-realistic model, it will also admit non-local models. The meaningful way to describe a local theory is to say that a theory is local when it admits a local model and conversely, a theory is non-local when it admits no local model.
Thus we can conclude that quantum theory is local-realistic since it has a local-realistic model.
Data accessibility. This article has no additional data. Competing interests. I declare I have no competing interests. Funding. This work has been supported in part by the Natural Sciences and Engineering Research Council of Canada, the Fonds de recherche du Québec-Nature et technologies and from Intesa Sanpaolo Innovation Center. The funders had no role in study design, data collection, and analysis, decision to publish, or preparation of the manuscript.