Quantum nonlocality

In theoretical physics, quantum nonlocality refers to the phenomenon by which the measurement statistics of a multipartite quantum system do not admit an interpretation in terms of a local realistic theory. Quantum nonlocality has been experimentally verified under different physical assumptions.[1][2][3][4][5] Any physical theory that aims at superseding or replacing quantum theory should account for such experiments and therefore must also be nonlocal in this sense; quantum nonlocality is a property of the universe that is independent of our description of nature.

Quantum nonlocality does not allow for faster-than-light communication,[6] and hence is compatible with special relativity. However, it prompts many of the foundational discussions concerning quantum theory, see Quantum foundations.

History

Einstein, Podolsky and Rosen

Main article: EPR paradox

In 1935, Einstein, Podolsky and Rosen published a thought experiment with which they hoped to expose the incompleteness of the Copenhagen interpretation of quantum mechanics in relation to the violation of local causality at the microscopic scale that it described.[7] Afterwards, Einstein presented a variant of these ideas in a letter to Erwin Schrödinger,[8] which is the version that is presented here. The state and notation used here are more modern, and akin to Bohm's take on EPR.[9] The quantum state of the two particles prior to measurement can be written as

${\displaystyle \left|\psi _{AB}\right\rangle ={\frac {1}{\sqrt {2}}}{\bigg (}\left|0\right\rangle _{A}\left|1\right\rangle _{B}-\left|1\right\rangle _{A}\left|0\right\rangle _{B}{\bigg )}={\frac {1}{\sqrt {2}}}{\bigg (}\left|+\right\rangle _{A}\left|-\right\rangle _{B}-\left|-\right\rangle _{A}\left|+\right\rangle _{B}{\bigg )}}$

where ${\displaystyle \left|\pm \right\rangle ={\frac {1}{\sqrt {2}}}\left(\left|0\right\rangle \pm \left|1\right\rangle \right)}$.[10]

Here, subscripts “A” and “B” distinguish the two particles, though it is more convenient and usual to refer to these particles as being in the possession of two experimentalists called Alice and Bob. The rules of quantum theory give predictions for the outcomes of measurements performed by the experimentalists. Alice, for example, will measure her particle to be spin-up in an average of fifty percent of measurements. However, according to the Copenhagen interpretation, Alice's measurement causes the state of the two particles to collapse, so that if Alice performs a measurement of spin in the z-direction, that is with respect to the basis ${\displaystyle \{\left|0\right\rangle _{A},\left|1\right\rangle _{A}\}}$, then Bob's system will be left in one of the states ${\displaystyle \{\left|0\right\rangle _{B},\left|1\right\rangle _{B}\}}$. Likewise, if Alice performs a measurement of spin in the x-direction, that is, with respect to the basis ${\displaystyle \{\left|+\right\rangle _{A},\left|-\right\rangle _{A}\}}$, then Bob's system will be left in one of the states ${\displaystyle \{\left|+\right\rangle _{B},\left|-\right\rangle _{B}\}}$. Schrödinger referred to this phenomenon as "steering".[11] This steering occurs in such a way that no signal can be sent by performing such a state update; quantum nonlocality cannot be used to send messages instantaneously and is therefore not in direct conflict with causality concerns in Special Relativity.[10]

In the Copenhagen view of this experiment, Alice's measurement—and particularly her measurement choice—has a direct effect on Bob's state. However, under the assumption of locality, actions on Alice's system do not affect the "true", or "ontic" state of Bob's system. We see that the ontic state of Bob's system must be compatible with one of the quantum states ${\displaystyle \left|\uparrow \right\rangle _{B}}$ or ${\displaystyle \left|\downarrow \right\rangle _{B}}$, since Alice can make a measurement that concludes with one of those states being the quantum description of his system. At the same time, it must also be compatible with one of the quantum states ${\displaystyle \left|\leftarrow \right\rangle _{B}}$ or ${\displaystyle \left|\rightarrow \right\rangle _{B}}$ for the same reason. Therefore, the ontic state of Bob's system must be compatible with at least two quantum states; the quantum state is therefore not a complete descriptor of his system. Einstein, Podolsky and Rosen saw this as evidence of the incompleteness of the Copenhagen interpretation of quantum theory, since the wavefunction is explicitly not a complete description of a quantum system under this assumption of locality. Their paper concludes:[7]

While we have thus shown that the wave function does not provide a complete description of the physical reality, we left open the question of whether or not such a description exists. We believe, however, that such a theory is possible.

Although various authors (most notably Niels Bohr) criticised the ambiguous terminology of the EPR paper,[12][13][13] the thought experiment nevertheless generated a great deal of interest. Their notion of a "complete description" was later formalised by the suggestion of hidden variables that determine the statistics of measurement results, but to which an observer does not have access.[14] Bohmian mechanics provides such a completion of quantum mechanics, with the introduction of hidden variables; however the theory is explicitly nonlocal.[15] The interpretation therefore does not give an answer to Einstein's question, which was whether or not a complete description of quantum mechanics could be given in terms of local hidden variables in keeping with the "Principle of Local Action".[16]

Probabilistic Nonlocality

See also: Bell test experiments

In 1964 John Bell answered Einstein's question by showing that such local hidden variables can never reproduce the full range of statistical outcomes predicted by quantum theory.[17] Bell showed that a local hidden variable hypothesis leads to restrictions on the strength of correlations of measurement results. If the Bell inequalities are violated experimentally as predicted by quantum mechanics, then reality cannot be described by local hidden variables and the mystery of quantum nonlocal causation remains. According to Bell:[17]

This [grossly nonlocal structure] is characteristic ... of any such theory which reproduces exactly the quantum mechanical predictions.

Clauser, Horne, Shimony and Holt (CHSH) reformulated these inequalities in a manner that was more conductive to experimental testing (see CHSH inequality).[18]

In the scenario proposed by Bell (a Bell scenario), two experimentalists, Alice and Bob, conduct experiments in separate labs. At each run, Alice (Bob) conducts an experiment ${\displaystyle x}$ ${\displaystyle (y)}$ in her (his) lab, obtaining outcome ${\displaystyle a}$ ${\displaystyle (b)}$. If Alice and Bob repeat their experiments several times, then they can estimate the probabilities ${\displaystyle P(a,b|x,y)}$, namely, the probability that Alice and Bob respectively observe the results ${\displaystyle a,b}$ when they respectively conduct the experiments x,y. In the following, each such set of probabilities ${\displaystyle \{P(a,b|x,y):a,b,x,y\}}$ will be denoted by just ${\displaystyle P(a,b|x,y)}$. In the quantum nonlocality slang, ${\displaystyle P(a,b|x,y)}$ is termed a box.[19]

Bell formalized the idea of a hidden variable by introducing the parameter ${\displaystyle \lambda }$ to locally characterize measurement results on each system:[17] "It is a matter of indifference ... whether λ denotes a single variable or a set ... and whether the variables are discrete or continuous". However, it is equivalent (and more intuitive) to think of ${\displaystyle \lambda }$ as a local "strategy" or "message" that occurs with some probability ${\displaystyle \rho (\lambda )}$ when Alice and Bob reboot their experimental setup. EPR's criteria of local separability then stipulates that each local strategy defines the distributions of independent outcomes if Alice conducts experiment x and Bob conducts experiment ${\displaystyle y}$:

${\displaystyle P(a,b|x,y,\lambda _{A},\lambda _{B})=P_{A}(a|s,\lambda _{A})P_{A}(a|s,\lambda _{A})}$

Here ${\displaystyle P_{A}(a|x,\lambda _{A})}$ (${\displaystyle P_{B}(b|y,\lambda _{B})}$) denotes the probability that Alice (Bob) obtains the result ${\displaystyle a}$ ${\displaystyle (b)}$ when she (he) conducts experiment ${\displaystyle x}$ ${\displaystyle (y)}$ and the local variable describing her (his) experiment has value ${\displaystyle \lambda _{A}}$ (${\displaystyle \lambda _{B}}$).

Suppose that ${\displaystyle \lambda _{A},\lambda _{B}}$ can take values from some set ${\displaystyle \Lambda }$. If each pair of values ${\displaystyle \lambda _{A},\lambda _{B}\in \Lambda }$ has an associated probability ${\displaystyle \rho (\lambda _{A},\lambda _{B})}$ of being selected (shared randomness is allowed, i.e., ${\displaystyle \lambda _{A},\lambda _{B}}$ can be correlated), then one can average over this distribution to obtain a formula for the joint probability of each measurement result:

${\displaystyle P(a,b|x,y)=\sum _{\lambda _{A},\lambda _{B}\in \Lambda }\rho (\lambda _{A},\lambda _{B})P_{A}(a|x,\lambda _{A})P_{B}(b|y,\lambda _{B})}$

A box admitting such a decomposition is called a Bell local or a classical box. Fixing the number of possible values which ${\displaystyle a,b,x,y}$ can each take, one can represent each box ${\displaystyle P(a,b|x,y)}$ as a finite vector with entries ${\displaystyle \left(P(a,b|x,y)\right)_{a,b,x,y}}$. In that representation, the set of all classical boxes forms a convex polytope. In the Bell scenario studied by CHSH, where ${\displaystyle a,b,x,y}$ can take values within ${\displaystyle {0,1}}$, any Bell local box ${\displaystyle P(a,b|x,y)}$ must satisfy the CHSH inequality:

${\displaystyle S_{CHSH}\equiv E(0,0)+E(1,0)+E(0,1)-E(1,1)\leq 2,}$

where

${\displaystyle E(x,y)\equiv \sum _{a,b=0,1}(-1)^{a+b}P(a,b|x,y).}$

The above considerations apply to model a quantum experiment. Consider two parties conducting local polarization measurements on a bipartite photonic state. The measurement result for the polarization of a photon can take one of two values (informally, whether the photon is polarized in that direction, or in the orthogonal direction). If each party is allowed to choose between just two different polarization directions, the experiment fits within the CHSH scenario. As noted by CHSH, there exist a quantum state and polarization directions which generate a box ${\displaystyle P(a,b|x,y)}$ with ${\displaystyle S_{CHSH}}$ equal to ${\displaystyle 2{\sqrt {2}}\approx 2.828}$. This demonstrates an explicit way in which a theory with ontological states that are local, with local measurements and only local actions cannot match the probabilistic predictions of quantum theory, disproving Einstein's hypothesis. Experimentalists such as Alain Aspect have verified the quantum violation of the CHSH inequality [1] as well as other formulations of Bell's inequality, to invalidate the local hidden variables hypothesis and confirm that reality is indeed nonlocal in the EPR sense.

Possibilistic Nonlocality

The demonstration of nonlocality due to Bell is probabilistic in the sense that it shows that the precise probabilities predicted by quantum mechanics for some entangled scenarios cannot be met by a local theory. (For short, here and henceforth "local theory" means "local hidden variables theory".) However, quantum mechanics permits an even stronger violation of local theories: a possibilistic one, in which local theories cannot even agree with quantum mechanics on which events are possible or impossible in an entangled scenario. The first proof of this kind was due to Greenberger, Horne and Zeilinger in 1993[20]

In 1993, Lucien Hardy demonstrated a logical proof of quantum nonlocality that, like the GHZ proof is a possibilistic proof.[21][22][23] The state involved is often called the GHZ state. It starts with the observation that the state ${\displaystyle \left|\psi \right\rangle }$ defined below can be written in a few suggestive ways:

${\displaystyle \left|\psi \right\rangle ={\frac {1}{\sqrt {3}}}\left(\left|00\right\rangle +\left|01\right\rangle +\left|10\right\rangle \right)={\frac {1}{\sqrt {3}}}\left({\sqrt {2}}\left|+0\right\rangle +{\frac {1}{\sqrt {2}}}\left(\left|+1\right\rangle +\left|-1\right\rangle \right)\right)={\frac {1}{\sqrt {3}}}\left({\sqrt {2}}\left|0+\right\rangle +{\frac {1}{\sqrt {2}}}\left(\left|1+\right\rangle +\left|1-\right\rangle \right)\right)}$

where, as above, ${\displaystyle |\pm \rangle ={\tfrac {1}{\sqrt {2}}}(\left|0\right\rangle \pm \left|1\right\rangle )}$.

The experiment consists of this entangled state being shared between two experimenters, each of whom has the ability to measure either with respect to the basis ${\displaystyle \{\left|0\right\rangle ,\left|1\right\rangle \}}$ or ${\displaystyle \{\left|+\right\rangle ,\left|-\right\rangle \}}$. We see that if they each measure with respect to ${\displaystyle \{\left|0\right\rangle ,\left|1\right\rangle \}}$, then they never see the outcome ${\displaystyle \left|11\right\rangle }$. If one measures with respect to ${\displaystyle \{\left|0\right\rangle ,\left|1\right\rangle \}}$ and the other ${\displaystyle \{\left|+\right\rangle ,\left|-\right\rangle \}}$, they never see the outcomes ${\displaystyle \left|-0\right\rangle ,}$ ${\displaystyle \left|0-\right\rangle .}$ However, sometimes they see the outcome ${\displaystyle \left|--\right\rangle }$ when measuring with respect to ${\displaystyle \{\left|+\right\rangle ,\left|-\right\rangle \}}$, since ${\displaystyle \langle --|\psi \rangle =-{\tfrac {1}{2{\sqrt {3}}}}\neq 0.}$

This leads to the paradox: having the outcome ${\displaystyle |--\rangle }$ we conclude that if one of the experimenters had measured with respect to the ${\displaystyle \{\left|0\right\rangle ,\left|1\right\rangle \}}$ basis instead, the outcome must have been ${\displaystyle |{-}1\rangle }$ or ${\displaystyle |1-\rangle }$, since ${\displaystyle |{-}0\rangle }$ and ${\displaystyle |0-\rangle }$ are impossible. But then, if they had both measured with respect to the ${\displaystyle \{\left|0\right\rangle ,\left|1\right\rangle \}}$ basis, by locality the result must have been ${\displaystyle \left|11\right\rangle }$, which is also impossible.

Nonlocal hidden variable models with a finite propagation speed

The work of Bancal et al.[24] generalizes Bell's result by proving that correlations achievable in quantum theory are also incompatible with a large class of superluminal hidden variable models. In this framework, faster-than-light signaling is precluded. However, the choice of settings of one party can influence hidden variables at another party's distant location, if there is enough time for a superluminal influence (of finite, but otherwise unknown speed) to propagate from one point to the other. In this scenario, any bipartite experiment revealing Bell nonlocality can just provide lower bounds on the hidden influence's propagation speed. Quantum experiments with three or more parties can, nonetheless, disprove all such non-local hidden variable models.[24]

Analogs of Bell’s theorem in more complicated causal structures

A simple Bayesian network. Rain influences whether the sprinkler is activated, and both rain and the sprinkler influence whether the grass is wet.

The random variables measured in a general experiment can depend on each other in complicated ways. In the field of causal inference, such dependencies are represented via Bayesian networks: directed acyclic graphs where each node represents a variable and an edge from a variable to another signifies that the former influences the latter and not otherwise, see the figure. In a standard bipartite Bell experiment, Alice's (Bob's) setting ${\displaystyle x}$ (${\displaystyle y}$), together with her (his) local variable ${\displaystyle \lambda _{A}}$ (${\displaystyle \lambda _{B}}$), influence her (his) local outcome ${\displaystyle a}$ (${\displaystyle b}$). Bell's theorem can thus be interpreted as a separation between the quantum and classical predictions in a type of causal structures with just one hidden node ${\displaystyle (\lambda _{A},\lambda _{B})}$. Similar separations have been established in other types of causal structures.[25] The characterization of the boundaries for classical correlations in such extended Bell scenarios is challenging, but there exist complete practical computational methods to achieve it.[26][27]

Entanglement and nonlocality

See also: Quantum entanglement

In the media and popular science, quantum nonlocality is often portrayed as being equivalent to entanglement. However, this is not the case. Quantum entanglement can be defined only within the formalism of quantum mechanics, i.e., it is a model-dependent property. In contrast, nonlocality refers to the impossibility of a description of observed statistics in terms of a local hidden variable model, so it is independent of the physical model used to describe the experiment.

It is true that for any pure entangled state there exists a choice of measurements that produce Bell nonlocal correlations, but the situation is more complex for mixed states. While any Bell nonlocal state must be entangled, there exist (mixed) entangled states which do not produce Bell nonlocal correlations[28] (although, operating on several copies of some of such states,[29] or carrying out local post-selections,[30] it is possible to witness nonlocal effects). In addition, reasonably simple examples of Bell inequalities have been found for which the quantum state giving the largest violation is never a maximally entangled state, showing that entanglement is, in some sense, not even proportional to nonlocality.[31][32][33]

Quantum correlations

As shown, the statistics achievable by two or more parties conducting experiments in a classical system are constrained in a non-trivial way. Analogously, the statistics achievable by separate observers in a quantum theory also happen to be restricted. The first derivation of a non-trivial statistical limit on the set of quantum correlations, due to B. Tsirelson,[34] is known as Tsirelson's bound. Consider the CHSH Bell scenario detailed before, but this time assume that, in their experiments, Alice and Bob are preparing and measuring quantum systems. In that case, the CHSH parameter can be shown to be bounded by

${\displaystyle -2{\sqrt {2}}\leq CHSH\leq 2{\sqrt {2}}.}$

The sets of quantum correlations and Tsirelson’s problem

Mathematically, a box ${\displaystyle P(a,b|x,y)}$ admits a quantum realization if and only if there exists a pair of Hilbert spaces ${\displaystyle H_{A},H_{B}}$, a normalized vector ${\displaystyle \left|\psi \right\rangle \in H_{A}\otimes H_{B}}$ and projection operators ${\displaystyle E_{a}^{x}:H_{A}\to H_{A},F_{b}^{y}:H_{B}\to H_{B}}$ such that

1. For all ${\displaystyle x,y}$, the sets ${\displaystyle \{E_{a}^{x}\}_{a},\{F_{b}^{y}\}_{b}}$ represent complete measurements. Namely, ${\displaystyle \sum _{a}E_{a}^{x}={\mathbb {I} }_{A},\sum _{b}F_{b}^{y}={\mathbb {I} }_{B}}$.
2. ${\displaystyle P(a,b|x,y)=\left\langle \psi \right|E_{a}^{x}\otimes F_{b}^{y}\left|\psi \right\rangle }$, for all ${\displaystyle a,b,x,y}$.

In the following, the set of such boxes will be called ${\displaystyle Q}$. Contrary to the classical set of correlations, when viewed in probability space, ${\displaystyle Q}$ is not a polytope. On the contrary, it contains both straight and curved boundaries.[35] In addition, ${\displaystyle Q}$ is not closed:[36] this means that there exist boxes ${\displaystyle P(a,b|x,y)}$ which can be arbitrarily well approximated by quantum systems but are themselves not quantum.

In the above definition, the space-like separation of the two parties conducting the Bell experiment was modeled by imposing that their associated operator algebras act on different factors ${\displaystyle H_{A},H_{B}}$ of the overall Hilbert space ${\displaystyle H=H_{A}\otimes H_{B}}$ describing the experiment. Alternatively, one could model space-like separation by imposing that these two algebras commute. This leads to a different definition:

${\displaystyle P(a,b|x,y)}$ admits a field quantum realization if and only if there exists a Hilbert space ${\displaystyle H}$, a normalized vector ${\displaystyle \left|\psi \right\rangle \in H}$ and projection operators ${\displaystyle E_{a}^{x}:H\to H,F_{b}^{y}:H\to H}$ such that

1. For all ${\displaystyle x,y}$, the sets ${\displaystyle \{E_{a}^{x}\}_{a},\{F_{b}^{y}\}_{b}}$ represent complete measurements. Namely, ${\displaystyle \sum _{a}E_{a}^{x}={\mathbb {I} },\sum _{b}F_{b}^{y}={\mathbb {I} }}$.
2. ${\displaystyle P(a,b|x,y)=\left\langle \psi \right|E_{a}^{x}F_{b}^{y}\left|\psi \right\rangle }$, for all ${\displaystyle a,b,x,y}$.
3. ${\displaystyle [E_{a}^{x},F_{b}^{y}]=0}$, for all ${\displaystyle a,b,x,y}$.

Call ${\displaystyle Q_{c}}$ the set of all such correlations ${\displaystyle P(a,b|x,y)}$.

How does this new set relate to the more conventional ${\displaystyle Q}$ defined above? It can be proven that ${\displaystyle Q_{c}}$ is closed. Moreover, ${\displaystyle Q_{c}\supset {\bar {Q}}}$, where ${\displaystyle {\bar {Q}}}$ denotes the closure of ${\displaystyle Q}$. Tsirelson's problem[37] consists in deciding whether the inclusion relation ${\displaystyle Q_{c}\supset {\bar {Q}}}$ is strict, i.e., whether or not ${\displaystyle Q_{c}={\bar {Q}}}$. This problem only appears in infinite dimensions: when the Hilbert space ${\displaystyle H}$ in the definition of ${\displaystyle Q_{c}}$ is constrained to be finite-dimensional, the closure of the corresponding set equals ${\displaystyle {\bar {Q}}}$.[37]

Tsirelson's problem can be shown equivalent to Connes embedding problem,[38][39][40] a famous conjecture in the theory of operator algebras.

Characterization of quantum correlations

Since the dimensions of ${\displaystyle H_{A}}$ and ${\displaystyle H_{B}}$ are, in principle, unbounded, determining whether a given box ${\displaystyle P(a,b|x,y)}$ admits a quantum realization is a complicated problem. In fact, the dual problem of establishing whether a quantum box can have a perfect score at a non-local game is known to be undecidable.[36] Moreover, the problem of deciding whether ${\displaystyle P(a,b|x,y)}$ can be approximated by a quantum system with precision ${\displaystyle 1/poly(|X||Y|)}$ is NP-hard.[41] Characterizing quantum boxes is equivalent to characterizing the cone of completely positive semidefinite matrices under a set of linear constraints.[42]

For small fixed dimensions ${\displaystyle d_{A},d_{B}}$, one can explore, using variational methods, whether ${\displaystyle P(a,b|x,y)}$ can be realized in a bipartite quantum system ${\displaystyle H_{A}\otimes H_{B}}$, with ${\displaystyle dim(H_{A})=d_{A}}$, ${\displaystyle dim(H_{B})=d_{B}}$. That method, however, can just be used to prove the realizability of ${\displaystyle P(a,b|x,y)}$, and not its unrealizability with quantum systems.

To prove unrealizability, the most known method is the Navascués-Pironio-Acín (NPA) hierarchy.[43] This is an infinite decreasing sequence of sets of correlations ${\displaystyle Q^{1}\supset Q^{2}\supset Q^{3}\supset ...}$ with the properties:

1. If ${\displaystyle P(a,b|x,y)\in Q_{c}}$, then ${\displaystyle P(a,b|x,y)\in Q^{k}}$ for all ${\displaystyle k}$.
2. If ${\displaystyle P(a,b|x,y)\not \in Q_{c}}$, then there exists ${\displaystyle k}$ such that ${\displaystyle P(a,b|x,y)\not \in Q^{k}}$.
3. For any ${\displaystyle k}$, deciding whether ${\displaystyle P(a,b|x,y)\in Q^{k}}$ can be cast as a semidefinite program.

The NPA hierarchy thus provides a computational characterization, not of ${\displaystyle Q}$, but of ${\displaystyle Q_{c}}$. If Tsirelson's problem is solved in the affirmative, namely, ${\displaystyle {\bar {Q}}=Q_{c}}$, then the above two methods would provide a practical characterization of ${\displaystyle {\bar {Q}}}$. If, on the contrary, ${\displaystyle {\bar {Q}}\not =Q_{c}}$, then a new method to detect the non-realizability of the correlations in ${\displaystyle Q_{c}-{\bar {Q}}}$ is needed.

The physics of supra-quantum correlations

The works listed above describe what the quantum set of correlations looks like, but they do not explain why. Are quantum correlations unavoidable, even in post-quantum physical theories, or on the contrary, could there exist correlations outside ${\displaystyle {\bar {Q}}}$ which nonetheless do not lead to any unphysical operational behavior?

In their seminal 1994 paper, Popescu and Rorhlich explore whether quantum correlations can be explained by appealing to relativistic causality alone.[44] Namely, whether any hypothetical box ${\displaystyle P(a,b|x,y)\not \in {\bar {Q}}}$ would allow building a device capable of transmitting information faster than the speed of light. At the level of correlations between two parties, Einstein's causality translates in the requirement that Alice's measurement choice should not affect Bob's statistics, and vice versa. Otherwise, Alice (Bob) could signal Bob (Alice) instantaneously by choosing her (his) measurement setting ${\displaystyle x}$ ${\displaystyle (y)}$ appropriately. Mathematically, Popescu and Rohrlich's no-signalling conditions are:

${\displaystyle \sum _{a}P(a,b|x,y)=\sum _{a}P(a,b|x^{\prime },y)=:P_{B}(b|y),}$

${\displaystyle \sum _{b}P(a,b|x,y)=\sum _{b}P(a,b|x,y^{\prime })=:P_{A}(a|x).}$

Like the set of classical boxes, when represented in probability space, the set of no-signalling boxes forms a polytope. Popescu and Rohrlich identified a box ${\displaystyle P(a,b|x,y)}$ that, while complying with the no-signalling conditions, violates Tsirelson's bound, and is thus unrealizable in quantum physics. Dubbed the PR-box, it can be written as:

${\displaystyle P(a,b|x,y)={\frac {1}{2}}\delta _{xy,a\oplus b}.}$

Here ${\displaystyle a,b,x,y}$ take values in ${\displaystyle {0,1}}$, and ${\displaystyle a\oplus b}$ denotes the sum modulo two. It can be verified that the CHSH value of this box is 4 (as opposed to the Tsirelson bound of ${\displaystyle 2{\sqrt {2}}\approx 2.828}$). This box had been identified earlier, by Rastall[45] and Khalfin and Tsirelson.[46]

In view of this mismatch, Popescu and Rohrlich pose the problem of identifying a physical principle, stronger than the no-signalling conditions, that allows deriving the set of quantum correlations. Several proposals followed:

1. Non-trivial communication complexity (NTCC).[47] This principle stipulates that nonlocal correlations should not be so strong as to allow two parties to solve all 1-way communication problems with some probability ${\displaystyle p>1/2}$ using just one bit of communication. It can be proven that any box violating Tsirelson's bound by more than ${\displaystyle 2{\sqrt {2}}\left({\frac {4}{\sqrt {3}}}-1\right)\approx 0.4377}$ is incompatible with NTCC.
2. No Advantage for Nonlocal Computation (NANLC).[48] The following scenario is considered: given a function ${\displaystyle f_{0,1}^{n}\to 1}$, two parties are distributed the strings of ${\displaystyle n}$ bits ${\displaystyle x,y}$ and asked to output the bits ${\displaystyle a,b}$ so that ${\displaystyle a\oplus b}$ is a good guess for ${\displaystyle f(x\oplus y)}$. The principle of NANLC states that non-local boxes should not give the two parties any advantage to play this game. It is proven that any box violating Tsirelson's bound would provide such an advantage.
3. Information Causality (IC).[49] The starting point is a bipartite communication scenario where one of the parts (Alice) is handed a random string ${\displaystyle x}$ of ${\displaystyle n}$ bits. The second part, Bob, receives a random number ${\displaystyle k\in \{1,...,n\}}$. Their goal is to transmit Bob the bit ${\displaystyle x_{k}}$, for which purpose Alice is allowed to transmit Bob ${\displaystyle s}$ bits. The principle of IC states that the sum over ${\displaystyle k}$ of the mutual information between Alice's bit and Bob's guess cannot exceed the number ${\displaystyle s}$ of bits transmitted by Alice. It is shown that any box violating Tsirelson's bound would allow two parties to violate IC.
4. Macroscopic Locality (ML).[50] In the considered setup, two separate parties conduct extensive low-resolution measurements over a large number of independently prepared pairs of correlated particles. ML states that any such “macroscopic” experiment must admit a local hidden variable model. It is proven that any microscopic experiment capable of violating Tsirelson's bound would also violate standard Bell nonlocality when brought to the macroscopic scale. Besides Tsirelson's bound, the principle of ML fully recovers the set of all two-point quantum correlators.
5. Local Orthogonality (LO).[51] This principle applies to multipartite Bell scenarios, where ${\displaystyle n}$ parties respectively conduct experiments ${\displaystyle x_{1},...,x_{n}}$ in their local labs. They respectively obtain the outcomes ${\displaystyle a_{1},...,a_{n}}$. The pair of vectors ${\displaystyle ({\bar {a}}|{\bar {x}})}$ is called an event. Two events ${\displaystyle ({\bar {a}}|{\bar {x}})}$, ${\displaystyle ({\bar {a}}^{\prime }|{\bar {x}}^{\prime })}$ are said to be locally orthogonal if there exists ${\displaystyle k}$ such that ${\displaystyle x_{k}=x_{k}^{\prime }}$ and ${\displaystyle a_{k}\not =a_{k}^{\prime }}$. The principle of LO states that, for any multipartite box, the sum of the probabilities of any set of pair-wise locally orthogonal events cannot exceed 1. It is proven that any bipartite box violating Tsirelson's bound by an amount of ${\displaystyle 0.052}$ violates LO.

All these principles can be experimentally falsified under the assumption that we can decide if two or more events are space-like separated. This sets this research program aside from the axiomatic reconstruction of quantum mechanics via Generalized Probabilistic Theories.

The works above rely on the implicit assumption that any physical set of correlations must be closed under wirings.[52] This means that any effective box built by combining the inputs and outputs of a number of boxes within the considered set must also belong to the set. Closure under wirings does not seem to enforce any limit on the maximum value of CHSH. However, it is not a void principle: on the contrary, in [52] it is shown that many simple, intuitive families of sets of correlations in probability space happen to violate it.

Originally, it was unknown whether any of these principles (or a subset thereof) was strong enough to derive all the constraints defining ${\displaystyle {\bar {Q}}}$. This state of affairs continued for some years until the construction of the almost quantum set ${\displaystyle {\tilde {Q}}}$.[53] ${\displaystyle {\tilde {Q}}}$ is a set of correlations that is closed under wirings and can be characterized via semidefinite programming. It contains all correlations in ${\displaystyle Q_{c}\supset {\bar {Q}}}$, but also some non-quantum boxes ${\displaystyle P(a,b|x,y)\not \in Q_{c}}$. Remarkably, all boxes within the almost quantum set are shown to be compatible with the principles of NTCC, NANLC, ML and LO. There is also numerical evidence that almost quantum boxes also comply with IC. It seems, therefore, that, even when the above principles are taken together, they do not suffice to single out the quantum set in the simplest Bell scenario of two parties, two inputs and two outputs.[53]

Device independent protocols

Nonlocality can be exploited to conduct quantum information tasks which do not rely on the knowledge of the inner workings of the prepare-and-measurement apparatuses involved in the experiment. The security or reliability of any such protocol just depends on the strength of the experimentally measured correlations ${\displaystyle P(a,b|x,y)}$. These protocols are termed device-independent.

Device-independent Quantum Key Distribution

Main article: Device-independent quantum cryptography

The first device-independent protocol proposed was device-independent Quantum Key Distribution (QKD).[54] In this primitive, two distant parties, Alice and Bob, are distributed an entangled quantum state, that they probe, thus obtaining the statistics ${\displaystyle P(a,b|x,y)}$. Based on how non-local the box ${\displaystyle P(a,b|x,y)}$ happens to be, Alice and Bob estimate how much knowledge an external quantum adversary Eve (the eavesdropper) could possess on the value of Alice and Bob's outputs. This estimation allows them to devise a reconciliation protocol at the end of which Alice and Bob share a perfectly correlated one-time pad of which Eve has no information whatsoever. The one-time pad can then be used to transmit a secret message through a public channel. Although the first security analyses on device-independent QKD relied on Eve carrying out a specific family of attacks,[55] all such protocols have been recently proven unconditionally secure.[56]

Device-independent randomness certification, expansion and amplification

Nonlocality can be used to certify that the outcomes of one of the parties in a Bell experiment are partially unknown to an external adversary.[57] By feeding a partially random seed to several non-local boxes, and, after processing the outputs, one can end up with a longer (potentially unbounded) string of comparable randomness[58] or with a shorter but more random string.[59] This last primitive can be proven impossible in a classical setting.[60]

Self-testing

Sometimes, the box ${\displaystyle P(a,b|x,y)}$ shared by Alice and Bob is such that it only admits a unique quantum realization. This means that there exist measurement operators ${\displaystyle E_{a}^{x},F_{b}^{y}}$ and a quantum state ${\displaystyle \left|\psi \right\rangle }$ giving rise to ${\displaystyle P(a,b|x,y)}$ such that any other physical realization ${\displaystyle {\tilde {E}}_{a}^{x},{\tilde {F}}_{b}^{y},\left|{\tilde {\psi }}\right\rangle }$ of ${\displaystyle P(a,b|x,y)}$ is connected to ${\displaystyle E_{a}^{x},F_{b}^{y},\left|\psi \right\rangle }$ via local unitary transformations. This phenomenon, that can be interpreted as an instance of device-independent quantum tomography, was first pointed out by Tsirelson [35] and named self-testing by Mayers and Yao.[54] Self-testing is known to be robust against systematic noise, i.e., if the experimentally measured statistics are close enough to ${\displaystyle P(a,b|x,y)}$, one can still determine the underlying state and measurement operators up to error bars.[54]

Dimension witnesses

The degree of non-locality of a quantum box ${\displaystyle P(a,b|x,y)}$ can also provide lower bounds on the Hilbert space dimension of the local systems accessible to Alice and Bob.[61] This problem is equivalent to deciding the existence of a matrix with low completely positive semidefinite rank.[62] Finding lower bounds on the Hilbert space dimension based on statistics happens to be a hard task, and current general methods only provide very low estimates.[63] However, a Bell scenario with five inputs and three outputs suffices to provide arbitrarily high lower bounds on the underlying Hilbert space dimension.[64] Quantum communication protocols which assume a knowledge of the local dimension of Alice and Bob's systems, but otherwise do not make claims on the mathematical description of the preparation and measuring devices involved are termed semi-device independent protocols. Currently, there exist semi-device independent protocols for quantum key distribution [65] and randomness expansion.[66]

See also

• Action at a distance
• Popper's experiment
• Quantum pseudo-telepathy
• Quantum contextuality
• Quantum foundations

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Further reading

• Grib, AA; Rodrigues, WA (1999). Nonlocality in Quantum Physics. Springer Verlag. ISBN 978-0-306-46182-8.
• Cramer, JG (2015). The Quantum Handshake: Entanglement, Nonlocality and Transactions. Springer Verlag. ISBN 978-3-319-24642-0.