The standard fair sampling assumption is not necessary to test local realism

# The standard fair sampling assumption is not necessary to test local realism

Dominic W. Berry, Hyunseok Jeong, Magdalena Stobińska, and Timothy C. Ralph Centre for Quantum Computer Technology, Macquarie University, Sydney, NSW 2109, Australia
Institute for Quantum Computing, University of Waterloo, Waterloo, ON N2L 3G1, Canada
Centre for Quantum Computer Technology, Department of Physics, The University of Queensland, St Lucia, Qld 4072, Australia
Center for Subwavelength Optics, Department of Physics and Astronomy, Seoul National University, Seoul, 151-742, Korea
Institut für Optik, Information und Photonik, Universität Erlangen-Nürnberg, Staudtstr. 7/B2, 91058 Erlangen, Germany
Institute of Theoretical Physics and Astrophysics, University of Gdańsk, ul. Wita Stwosza 57, 80-952 Gdańsk, Poland
###### Abstract

Almost all Bell-inequality experiments to date have used postselection, and therefore relied on the fair sampling assumption for their interpretation. The standard form of the fair sampling assumption is that the loss is independent of the measurement settings, so the ensemble of detected systems provides a fair statistical sample of the total ensemble. This is often assumed to be needed to interpret Bell inequality experiments as ruling out hidden-variable theories. Here we show that it is not necessary; the loss can depend on measurement settings, provided the detection efficiency factorises as a function of the measurement settings and any hidden variable. This condition implies that Tsirelson’s bound must be satisfied for entangled states. On the other hand, we show that it is possible for Tsirelson’s bound to be violated while the CHSH-Bell inequality still holds for unentangled states, and present an experimentally feasible example.

###### pacs:
03.65.Ud,03.67.-a,03.65.Ta

## I Introduction

When quantum mechanics was first developed it was argued that it might only be an approximation of an underlying classical “hidden-variable” theory epr (). This was put on a testable basis by the development of Bell inequalities bell (); chsh (); ch74 (), which should be obeyed by any local hidden variable (LHV) theory. Experimental violation freedman (); aspect (); shih (); ou (); rarity (); tittel (); weihs (); kwiat (); rowe (); moehring (); matsukevich () of Bell inequalities provides strong evidence against LHV theories, but almost all of these experiments (with the exceptions of those in Refs. rowe (); matsukevich ()) have the loophole that the violation of the Bell inequality could, in principle, be caused by loss lo (); pearle (); garg (); santos (); eber (); gisin (). The interpretation of these experiments as ruling out LHV theories therefore relies on the assumption that the sampling is “fair” chsh (); fair (). For the interpretation of these experiments it is therefore vital to establish what constitutes fair sampling. Here we put fair sampling on a rigorous basis by determining exactly what forms of loss can lead to violation of Bell inequalities.

The standard form of the fair sampling assumption is that the detection efficiency is independent of measurement settings chsh (); fair (). Here we find that assumption is unnecessary. The efficiency can depend on the measurement settings, provided the efficiency factorises as a function of the measurement settings and any hidden variable. Most experimental tests are of the Clauser, Horne, Shimony and Holt (CHSH) form of the Bell inequality chsh (), and we therefore concentrate on the CHSH-Bell inequality in this work. Our condition is both necessary and sufficient for the CHSH-Bell inequality to be satisfied for LHV theories. An alternative sufficient condition was previously found by Ref. shaf (). We also establish the necessary and sufficient condition for the CHSH-Bell inequality to be satisfied for unentangled states, and show that if the sampling is fair it will also prevent violation of Tsirelson’s bound tsirelson () with entangled states.

This result means that, in order to obtain violation of Tsirelson’s bound tsirelson () with entangled states, but not of the CHSH-Bell inequality with unentangled states, it is necessary to examine the specific measurement, and not just the form of the loss. We present a scheme that violates Tsirelson’s bound with entangled states, but not the CHSH-Bell inequality with unentangled states. The CHSH-Bell inequality is still violated with LHV theories, but the scheme can tolerate greater loss than the bound derived in Ref. garg (). Other methods of constructing Bell inequalities with greater resistance to loss have been proposed in Refs. eber (); massar (); durt (); genovese (); brun ().

This manuscript is organised as follows. First the fair sampling assumption is explained in more detail in Sec. II. General Bell inequalities are presented in Sec. III, then postselection for local hidden variable theories is analysed in Sec. IV. Postselection for quantum mechanics, including Tsirelson’s bound, is analysed in Sec. V. The use of postselection to enhance violation of Bell inequalities beyond Tsirelson’s bound for entangled states is analysed in Sec. VI. We conclude in Sec. VII.

## Ii The fair sampling assumption

The first work to give a form of the fair sampling assumption was that of Clauser, Horne, Shimony and Holt chsh (). They assumed, in deriving their inequality, that the detection efficiency is independent of the measurement settings. Pearle expressed the assumption alternatively, that “the data recorded [is] representative of the accepted data” pearle (). That is, that the sample of detected pairs provides a fair statistical sample of all the pairs. These forms of the fair sampling assumption, which superficially appear different, are effectively equivalent.

For the sample to be completely fair, the probability of sampling a pair (i.e. the efficiency) needs to be independent of the pair. For this to be the case, the efficiency needs to be independent of any quantity that varies between the individual pairs. The only quantities that can vary between the individual pairs are the internal state (the quantum state or any hypothetical hidden variable) and the measurement setting that is used in measuring the pair. Therefore the requirement that the sample is fair is exactly equivalent to requiring the efficiency to be independent of the internal state and measurement setting.

This requirement is slightly stronger than the requirement given by Ref. chsh (), because it requires that the efficiency is also independent of the state of the pair. However, it is easily seen that the efficiency need not be independent of the state. This is because, if the efficiency is dependent on the state, but independent of the measurement setting, then the postselection simply changes the probabilities for the internal state, yielding a different postselected state. That is, the sampling may not be fair, but the loss is simply yielding a postselected state on which the sampling is fair.

This is taken advantage of in Procrustean entanglement concentration Bennett (), which has been demonstrated to enhance the violation of Bell inequalitites Kwiat01 (). Procrustean entanglement concentration gives loss that depends on the state, but because this loss is independent of the measurement settings of the Bell measurement, it does not invalidate the Bell inequalities for unentangled states. Although the sampling is not entirely fair for the initial state, it is fair for the state produced by the Procrustean entanglement concentration.

It is important to note that the condition that the efficiency is independent of the measurement setting means that it must be completely independent of the measurement setting. That is, it can not be a function of the measurement setting, so it is independent of the measurement setting for any internal state. On the other hand, if the efficiency is independent of the measurement setting for just one state, then it is easy to provide examples where the Bell inequality is violated with unentangled states or hidden variables. For a simple example, see Appendix A.

## Iii General Bell inequalities

In a general Bell inequality experiment with multiple parties, these parties each share one component of a state , and each performs one of a number of different measurements. The measurement settings for party are denoted , and the measurement results are denoted . We denote the vectors of measurement settings and measurement results and . One obtains a set of measurement probabilities , and can define a Bell quantity as a linear combination of these probabilities. A Bell inequality is then an upper bound on the value of this quantity for LHV theories. With loss, we denote the probability of a successful measurement for settings by . The postselected probabilities are then given by

 ~p(→s|→γ,ρ)=p(→s|→γ,ρ)/E(→γ,ρ). (1)

We do not consider complete loss, which would make the postselected probabilities undefined.

In the specific case of CHSH-Bell inequalities, there are two parties, Alice and Bob, and each performs one of two dichotomic measurements. Now using the notation and for the measurement settings for Alice and Bob, respectively, we have , , and . The CHSH-Bell quantity without postselection is defined by

 B0:=C(A,B)+C(A,b)+C(a,B)−C(a,b), (2)

where

 C(α,β) :=p(+,+|α,β,ρ)−p(+,−|α,β,ρ) −p(−,+|α,β,ρ)+p(−,−|α,β,ρ). (3)

The postselected form of the CHSH-Bell quantity is

 B:=C(A,B)E(A,B,ρ)+C(a,B)E(a,B,ρ)+C(A,b)E(A,b,ρ)−C(a,b)E(a,b,ρ). (4)

## Iv Local hidden-variable theories

First we prove that Bell inequalities must be satisfied for LHV theories provided the detection efficiency factorises as a function of the measurement setting and a function of the hidden variable. For a stochastic local hidden-variable theory, probabilities are given as

 p(→s|→γ,ρ)=∑xp(x|ρ)∏kpk(sk|γk,x), (5)

where is the hidden variable. The state simply controls the probability distribution for . With loss, the probabilities can sum to less than 1. Summing over the measurement results gives the efficiencies as

 E(→γ,ρ)=∑xp(x|ρ)∏kEk(γk,x), (6)

where is the single-party efficiency for party with measurement setting and hidden variable .

We also use the notation for the efficiency due to measurement setting for party , and for the efficiency due to the hidden variable for party . With this notation defined, we can now state our condition rigorously.

###### Theorem 1.

When the efficiency for each party factorises as

 Ek(γk,x) =EkS(γk)EkH(x), (7)

the set of postselected probabilities that can be obtained is identical to that which can be obtained without postselection (provided no efficiency is zero).

This result means that this form of loss does not change the type of probability distributions that are possible with LHV models, and in particular any Bell inequality must still be satisfied with postselection.

###### Proof.

The proof follows by showing that there exists a measurement scheme without postselection that yields the same probabilities as the for the postselected scheme. The postselected probabilities may alternatively be given by

 ~p(→s|→γ,ρ)=∑x~p(x|ρ)∏k~p(sk|γk,x), (8)

where

 ~p(x|ρ) =p(x|ρ)ER(ρ)∏kEkH(x), ER(ρ) =∑xp(x|ρ)∏kEkH(x), ~p(sk|γk,x) =p(sk|γk,x)/Ek(γk,x). (9)

This means that, by using a different LHV model with different probabilities, we may obtain exactly the same probability distribution for the measurement results as for the postselected case. ∎

This result shows that our condition (7) is sufficient for Bell inequalities to hold with postselection. We also have a necessity proof in the case of CHSH-Bell inequalities. Before showing this result, we first show the general form of the CHSH-Bell inequality with postelection.

###### Lemma 1.

Any local hidden variable theory must satisfy

 |B|≤4−2∑xp(x|ρ)minαx,βxE1(αx,x)E2(βx,x)E(αx,βx,ρ). (10)

For given there exist probabilities that saturate this inequality.

Here we have used the same notation as for general Bell inequalities, except we have used and for Alice and Bob’s measurement settings, respectively. We use the superscript on and to indicate that these are chosen as a function of the hidden variable .

###### Proof.

For a LHV theory, the postselected CHSH-Bell quantity can be rewritten as

 B =∑xp(x|ρ){Δ1(A,x)Δ2(B,x)E(A,B,ρ)+Δ1(a,x)Δ2(B,x)E(a,B,ρ) +Δ1(A,x)Δ2(b,x)E(A,b,ρ)−Δ1(a,x)Δ2(b,x)E(a,b,ρ)}, (11)

where

 Δk(γk,x)=pk(+|γk,x)−pk(−|γk,x).

Because the probabilities are non-negative, we have . Considering arbitrary measurements for a given form of loss, we can choose the such that takes any value in the range .

Because is linear in each of the , it is maximised (or minimised) by taking extreme values where . By appropriately choosing the signs, it is possible to make any one of the terms in the curly brackets in Eq. (IV) negative, and the rest positive. Changing the sign preserves the parity of the number of negative terms, so it is not possible to make all terms positive.

In particular, taking makes the last term negative. Then changing to makes only the third term negative. Alternatively, changing to makes only the second term negative, or changing to and to makes only the first term negative.

To maximise , we take three terms positive and one negative for each value of . The value of will be maximised with the smallest term taken to be negative. That is,

 B =∑xp(x|ρ){E1(A,x)E2(B,x)E(A,B,ρ)+E1(a,x)E2(B,x)E(a,B,ρ) +E1(A,x)E2(b,x)E(A,b,ρ)+E1(a,x)E2(b,x)E(a,b,ρ) −2minαx,βxE1(αx,x)E2(βx,x)E(αx,βx,ρ)}. (12)

Summing the first four terms in Eq. (IV) gives equal to

 Bmax=4−2∑xp(x|ρ)minαx,βxE1(αx,x)E2(βx,x)E(αx,βx,ρ). (13)

To change the overall sign, so one term is positive and the remaining are negative, we can change the sign of both and . Using this, we can ensure that the largest three terms in Eq. (IV) positive, and the smallest is positive. Doing this for each value of , we simply obtain the negative of what was obtained before, and so obtain . We therefore find that the generalisation of the CHSH-Bell inequality for the case of postselection is , as given in Eq. (10). As the above argument is constructive, it shows how to choose probabilities in order to saturate this inequality. ∎

Using this result, we can prove the necessary and sufficient condition for the CHSH-Bell inequality to hold for LHV theories with postselection. We first prove the necessary and sufficient condition in an alternative form.

###### Lemma 2.

The condition that

 E1(α,x)E2(β,x)E(α,β,ρ) (14)

is independent of and is necessary and sufficient for to be satisfied for all probabilities .

###### Proof.

In order for to satisfy the usual CHSH-Bell inequality, , the sum in Eq. (10) must be equal to 1. Given that the condition is satisfied, we may take and for some arbitrary and in Eq. (10), giving

 |B|≤4−2∑xp(x|ρ)E1(α,x)E2(β,x)E(α,β,ρ)=2. (15)

Thus the condition is sufficient.

To prove necessity, we show that if the condition in Lemma 2 is not satisfied, then may be violated. If the condition is not satisfied for , then select and such that

 E1(α,z)E2(β,z)E(α,β,ρ)>E1(αz,z)E2(βz,z)E(αz,βz,ρ). (16)

We than have

 ∑xp(x|ρ)E1(αx,x)E2(βx,x)E(αx,βx,ρ) ≤∑xp(x|ρ)E1(α,x)E2(β,x)E(α,β,ρ) −p(z|ρ)(E1(α,z)E2(β,z)E(α,β,ρ)−E1(αz,z)E2(βz,z)E(αz,βz,ρ)) <1. (17)

As there exists a choice of probabilities which saturate the inequality (10), we can obtain . Hence we may obtain if the condition in Lemma 2 is violated, and it is therefore a necessary condition. ∎

We can now use Lemma 2 to show that the factorisation condition (7) is sufficient and necessary for the CHSH-Bell inequality. Specifically, we have the following theorem.

###### Theorem 2.

The condition that the efficiency for each party factorises as

 Ek(γk,x)=EkS(γk)EkH(x), (18)

is necessary and sufficient for to be satisfied for all probabilities (provided no efficiency is zero).

###### Proof.

The proof proceeds simply by showing that the condition in Lemma 2 is equivalent to (18). First, it is trivial to show that Eq. (18) implies the condition. Using Eq. (18) gives

 E1(α,x)E2(β,x)E(α,β,ρ)=E1H(x)E2H(x)ER(ρ), (19)

which is independent of and .

To show that the condition of Lemma 2 implies (18), we simply need to use it to define the quantities and . Let us define, for some ,

 E1S(α) :=E1(α,x0)/maxα′E1(α′,x0), (20) E1H(x) :=maxαE1(α,x), (21) E2S(β) :=E2(β,x0)/maxβ′E1(β′,x0), (22) E2H(x) :=maxβE1(β,x). (23)

It remains to show that these definitions satisfy (18). We find that

 E1S(α)E2S(β) =E1(α,x0)E2(β,x0)maxα,βE1(α,x0)E1(β,x0) =E(α,β,ρ)maxα,βE(α,β,ρ), (24)

where in the second line we use the condition of Lemma 2, and may be arbitrary. Hence we find that is independent of , and we therefore have

 E1S(α)E1H(x)E2S(β)E2H(x)=E1(α,x)E2(β,x). (25)

Rearranging Eq. (25) to isolate gives

 E1(α,x)=E1S(α)E1H(x)E2S(β)E2H(x)E2(β,x). (26)

Taking the maximum over then yields

 E1H(x)=E1H(x)E2S(β)E2H(x)E2(β,x), (27)

where we have used . Hence

 E2(β,x)=E2S(β)E2H(x). (28)

Using this expression in Eq. (25) gives

 E1(α,x)=E1S(α)E1H(x). (29)

Thus we have shown that the definitions (20) to (23) satisfy Eq. (18) provided the condition of Lemma 2 holds.

Hence we have shown that the condition of Lemma 2 and the condition (18) are equivalent, and therefore Theorem 2 follows from Lemma 2. ∎

## V Quantum mechanics

Next we consider the restriction on the loss for quantum mechanics, rather than LHV theories. It might be thought that the case of quantum mechanics is equivalent, because a LHV theory can be thought of as an unentangled state, with the labeling orthogonal basis states. However, the case of quantum mechanics is slightly different, because we also need to consider all linear combinations of orthogonal basis states.

For quantum theory the probabilities of local measurement results are obtained via a positive operator-valued measure with elements , which corresponds to successful measurement result for measurement setting for party . We also use the notation

 Mk,γk:=∑skMskk,γk, (30)

for the operator corresponding to a successful measurement. Here the sum is over all successful measurement results ; the measurement operator for failure is .

The restriction on the loss in terms of hidden variables (7) implies that

 E(→γ,ρ)=ER(ρ)∏kEkS(γk). (31)

This expression may be taken to be the definition of the restriction on the loss for quantum mechanics. This restriction may alternatively be expressed as

 Tr[(⨂kMk,γk)ρ]=ER(ρ)∏kEkS(γk). (32)

Let

 M:=⨂kMk,γk∏kEkS(γk). (33)

The restriction (32) implies that independent of , and therefore is independent of . This is why no subscript is given for . Thus the restriction in Eq. (31) implies that the are independent of .

Using a similar method as for hidden variables, we can show that postselection with this form of loss cannot change the form of probability distributions obtained, either for the case of entangled or unentangled states. In particular, the result is as in the following theorem.

###### Theorem 3.

For a Bell experiment on a quantum mechanical system, provided the loss is restricted by

 p(→γ,ρ)=ER(ρ)∏kEkS(γk), (34)

the set of postselected probabilities it is possible to obtain without entanglement is identical to that which can be obtained without postselection or entanglement, and the set of postselected probabilities it is possible to obtain with entanglement is identical to that which can be obtained without postelection but with entanglement (provided no efficiency is zero).

###### Proof.

We define new measurement operators as

 ~M±k,γk:=(Mk,γk)−1/2Mskk,γk(Mk,γk)−1/2. (35)

These measurement operators now give unit efficiency (so there is no postselection). We also define

 ~ρ:=M−1/2ρM−1/2Tr(M−1/2ρM−1/2), (36)

where is defined as in Eq. (33). Because we restrict to the case of incomplete loss, the measurement operators are positive and can be inverted. The new measurement operators and states give exactly the same probabilities without postselection as the original measurement operators and states did with postselection.

Furthermore, because is a local operator, it can not produce entangled states from unentangled states. Therefore the postselected Bell experiment with an unentangled state gives postselected probabilities identical to the non-postselected probabilities for a different Bell experiment with different measurement operators and a different unentangled state . ∎

This result means that, for an unentangled state, all Bell inequalities must still be satisfied. This is exactly as we expect, because unentangled states may be regarded as equivalent to hidden variables. Similarly, inequalities that hold for entangled states (such as Tsirelson’s bound) will be unaffected by the postselection.

For CHSH-Bell inequalities, it would be expected that Eq. (32) is also a necessary condition due to the result for hidden-variable theories. However, it does not directly follow, and necessity needs to be proven separately. This is because one cannot arbitrarily choose the probabilities for given efficiencies. Therefore it is not necessarily possible to achieve the maximum value of Eq. (10), as in the case of a general hidden-variable theory. Nevertheless, it is possible to show the result in the following theorem.

###### Theorem 4.

For a quantum mechanical system, the condition that the efficiency for each party factorises as

 E(→γ,ρ)=ER(ρ)∏kEkS(γk), (37)

is necessary and sufficient for to be satisfied for all probabilities (provided no efficiency is zero).

###### Proof.

The sufficiency follows immediately from Theorem 3, so it only remains to show necessity. The condition in the theorem is equivalent to Eq. (32), so we show necessity for Eq. (32). First consider the case where Eq. (32) is violated. In that case, either is dependent on , or is dependent on (or both). We omit the subscripts and in the notation and for simplicity. The party is simply indicated by the symbol used for the measurement setting ( for party 1 and for party 2).

If (for example) is not independent of , then there exist orthogonal states and such that

 ⟨φ0|Ma|φ0⟩⟨φ1|MA|φ1⟩≠⟨φ0|MA|φ0⟩⟨φ1|Ma|φ1⟩. (38)

This result may be proven in the following way. Let us assume that all orthogonal states give equality in (38). Then, for any orthogonal basis , we have

 ⟨φj|Ma|φj⟩=κ⟨φj|MA|φj⟩, (39)

for some . Therefore . Now we can take to be the basis which diagonalises . Then we have

 ⟨φ′j|Ma|φ′j⟩=κ′⟨φ′j|MA|φ′j⟩, (40)

so . Because is nonzero (these are positive operators), we have . Therefore the diagonal elements of must be zero in the basis . As this is the basis which diagonalises , we must have . Hence we find that equality in (38) implies , so if is not proportional to , then there must exist orthogonal states and such that (38) is satisfied.

We obtain the exact equivalent result if is not independent of . Therefore, if Eq. (32) is violated, we can select and such that

 ⟨φ0|Ma|φ0⟩⟨φ1|MA|φ1⟩ ≤⟨φ0|MA|φ0⟩⟨φ1|Ma|φ1⟩, ⟨χ0|Mb|χ0⟩⟨χ1|MB|χ1⟩ ≤⟨χ0|MB|χ0⟩⟨χ1|Mb|χ1⟩, (41)

with strict inequality in at least one of these cases. We therefore have

 ⟨φ0|Ma|φ0⟩⟨φ1|MA|φ1⟩⟨χ0|Mb|χ0⟩⟨χ1|MB|χ1⟩ <⟨φ0|MA|φ0⟩⟨φ1|Ma|φ1⟩⟨χ0|MB|χ0⟩⟨χ1|Mb|χ1⟩. (42)

Now consider the density operator

 ρ=(|φ0⟩⟨φ0|⊗|χ0⟩⟨χ0|+|φ1⟩⟨φ1|⊗|χ1⟩⟨χ1|)/2. (43)

For this density operator

 B =121∑j=0(⟨ΔMA⟩j⟨ΔMB⟩jTr[(MA⊗MB)ρ]+⟨ΔMA⟩j⟨ΔMb⟩jTr% [(MA⊗Mb)ρ] +⟨ΔMa⟩j⟨ΔMB⟩jTr[(Ma⊗MB)ρ]−⟨ΔMa⟩j⟨ΔMb⟩jTr[(Ma⊗Mb)ρ]), (44)

where , and indicates the expectation value using the state (for Alice) or (for Bob). Given the , consider the measurement operators for the individual results given by

 M+A =MA,M+a=|φ0⟩⟨φ0|⟨Ma⟩0, M−A =0,M−a=Ma−|φ0⟩⟨φ0|⟨Ma⟩0, M+B =|φ0⟩⟨φ0|⟨MB⟩0,M+b=MB, M−B =MB−|φ0⟩⟨φ0|⟨MB⟩0,M−b=0. (45)

Using these measurement operators gives

 ⟨ΔMa⟩j =(−1)j⟨Ma⟩j,⟨ΔMA⟩j=⟨MA⟩j, ⟨ΔMb⟩j =⟨Mb⟩j,⟨ΔMB⟩j=(−1)j⟨MB⟩j. (46)

This gives the postselected Bell quantity as

 B =4−2⟨Ma⟩0⟨Mb⟩0⟨Ma⟩0⟨Mb⟩0+⟨Ma⟩1⟨Mb⟩1 −2⟨MA⟩1⟨MB⟩1⟨MA⟩0⟨MB⟩0+⟨MA⟩1⟨MB⟩1. (47)

Equation (V) may be rearranged to give

 ⟨Ma⟩0⟨Mb⟩0⟨Ma⟩0⟨Mb⟩0+⟨Ma⟩1⟨Mb⟩1 +⟨MA⟩1⟨MB⟩1⟨MA⟩0⟨MB⟩0+⟨MA⟩1⟨MB⟩1<1. (48)

We therefore obtain .

Thus we find that, if Eq. (31) is not satisfied, for given there exists a separable state and a set of measurement operators such that . Eq. (31) is therefore a necessary condition for the CHSH-Bell inequality to be satisfied for separable states. As Eq. (31) is equivalent to the condition in the theorem, we have proven both necessity and sufficiency as required. ∎

For entangled states, is limited by Tsirelson’s bound of tsirelson (). As explained above, the restriction given by Eq. (31) is sufficient for Tsirelson’s bound to be satisfied due to the result in Theorem 3. However, it turns out that it is not necessary. In particular, we find that Tsirelson’s bound is not violated if there is no loss on one side, and moderate loss on the other side. Let , and let

 MB=[100p]. (49)

We have performed numerical maximisations over the measurements and states for a range of values of , and the results are shown in Fig. 1. For small values of , below about , there is violation of Tsirelson’s bound, but for larger values no violation of Tsirelson’s bound is achieved. This indicates that there is not a simple necessary and sufficient condition in the case of Tsirelson’s bound. Whether Tsirelson’s bound can be violated depends on the particular value of the loss.

An interesting fact is that if the condition (31) is violated for both parties, in the sense that is dependent on for both Alice and Bob, then it is always possible to find measurements such that Tsirelson’s bound is violated. A scheme for doing this is presented in Appendix B.

## Vi Postselection that violates Tsirelson’s bound

A central motivation for this work was to determine forms of loss that can violate Tsirelson’s bound while ensuring that the CHSH-Bell inequality is still valid, in order to generalise Ref. cab (). The result of the previous section is that the form of postselection that is necessary for the CHSH-Bell inequality to hold for unentangled states (as shown in Theorem 4) also implies that Tsirelson’s bound holds for entangled states (as follows from Theorem 3).

This raises the question of how the postselection in Ref. cab () differs from the postselection used here. The difference is that the postselection relies on the experimenter knowing what the state is. This method for constructing Bell inequalities is criticised in Ref. anne (), because it introduces an additional assumption beyond locality and realism. If an entangled state is incorrectly assumed, but the actual state is unentangled, then the method of Ref. cab () still yields a violation of the Bell inequality (See Appendix C). We therefore avoid the approach of assuming a state here, and simply allow postselection that may depend on the state and measurement setting.

A crucial subtlety in our results is that the condition (31) is necessary for the CHSH-Bell inequality to be satisfied for unentangled states, provided we consider arbitrary measurement schemes for the given form of loss. This does not eliminate the possibility that there are particular measurement schemes with postselection such that the Bell inequality is satisfied for unentangled states but Tsirelson’s bound may be violated for entangled states. We consider such a scheme in this section.

We emphasise that this scheme does not violate the Bell inequality with unentangled states provided the measurements are acting as expected. But, if there is an underlying hidden variable theory, or equivalently if the measurements are not acting as expected on the underlying quantum state, then the CHSH-Bell inequality can be violated without entanglement.

The advantage of this postselection is that it also increases the Bell quantity that may be obtained with entanglement. The standard result that the efficiency must be at least with maximally entangled states garg () is based upon the assumption that Tsirelson’s bound still holds for entangled states. If the Bell quantity is also enhanced for entangled states, then the efficiency may be lower before the value that is possible with a LHV theory reaches that possible with entangled states.

The example we consider is where Alice and Bob share the two-qubit entangled state

 |ψ−⟩12=N(|u⟩1|u⟩2−|v⟩1|v⟩2) (50)

where is the normalisation factor. The states and are assumed to be non-orthogonal, with the real inner product . We define a local transformation which acts as and .

The transformation is non-unitary and cannot be realised deterministically with a nonzero . Alice performs the local operation , and Bob applies . The different measurement settings for Alice and Bob are achieved by using different rotation angles and . This non-deterministically transforms the state to

 |ψ′−⟩12=N′(|u⟩1|u⟩2−ei(θ+ϕ)|v⟩1|v⟩2). (51)

Alice and Bob then perform orthogonal measurements on their respective qubits using the basis , and there are four possible cases of the combined measurement results. The probabilities for these four cases are

 P++(θ,ϕ) =(1+κ)2(1−cos[θ+ϕ])4(1−κ2cos[θ+ϕ]), P+−(θ,ϕ) =P−+(θ,ϕ)=(1−κ2)(1+cos[θ+ϕ])4(1−κ2cos[θ+ϕ]), P−−(θ,ϕ) =(1−κ)2(1−cos[θ+ϕ])4(1−κ2cos[θ+ϕ]), (52)

where .

The Bell function is then obtained as

 B=C(θA,ϕB)+C(θA,ϕb)+C(θa,ϕB)−C(θa,ϕb), (53)

where

 C(θ,ϕ) =P++−P+−−P−++P−− =κ2−cos(θ+ϕ)1−κ2cos(θ+ϕ). (54)

The maximum is obtained for

 (θA+θa+ϕB+ϕb)=θa−θA=ϕb−ϕB=Θ, (55)

for some parameter . The Bell function then depends only on :

 B=3C(Θ/2,0)−C(3Θ/2,0). (56)

There does not appear to be an analytic solution for , but a good approximation is given by .

To determine the loss that is required for the operation on and , consider the singular value decomposition SVD () of the matrix representing , i.e., (omitting a global phase) where

 U±=1√b2+(r±d)2[∗10cc−ibr±d−(r±d)ib], (57) W=⎡⎢ ⎢⎣√a−r20,0√a+r2⎤⎥ ⎥⎦, (58)

with , , , and . This therefore gives the minimum detector efficiency as

 η=√a−ra+r. (59)

The maximum value of possible with LHV theories is then garg ().

The values of the quantity for the initial state , as well as the maximum values for separable states, and the maximum values for LHV theories, are plotted in Fig. 2. The maximum value for separable states was obtained by numerical optimisation, and the maximum value for LHV theories was obtained using the formula . For , the value for entangled states varies from Tsirelson’s bound for to a maximum of 4 in the limit . On the other hand, initially has a maximum of for separable states. It increases with , but still does not exceed 2 for . For this value of , is almost 3 (2.966) for . On the other hand, the maximum value of for LHV theories increases from 2 for (no loss), and crosses the line for entangled states at . At this value of , , slightly below the limit of derived in Ref. garg ().

We have also considered more general measurements that do not have the simple interpretation given above. These measurements are numerically optimised to maximise the value of for entangled states with a given level of loss. The results for this scheme are shown in Fig. 3. For this numerically optimised scheme the value of can be greater than 3 (3.0046) for entangled states before it reaches 2 for separable states. The value of when the value of for LHV theories reaches that for entangled states is slightly lower than before, at .

Methods for general non-unitary transformations such as have been presented in Ref. tera05 (), and methods for performing single-qubit non-unitary transformations in optical systems in Ref. bergou00 (). An experiment for our proposal can be performed using current technology with the photon-polarisation qubit basis, namely, and where is the horizontal-polarisation state of a photon and vertical. The two non-orthogonal states and can be defined as and , where is assumed to be a real value larger than . In this case, the orthogonal basis states, and , are obtained and . The entangled state turns out to be equal to . It is well known that such a two-qubit entangled state can be generated using spontaneous parametric down-conversion Kwiat95 ().

Via a singular value decomposition, may be expressed as , where the are unitary and is diagonal, as given in Eqs. (57) and (58), respectively. The unitary operations correspond to single qubit rotations, and can be implemented using linear optical elements KLM (). After is performed on the corresponding qubit, the non-unitary component can be achieved using selective absorption at one polarisation. Provided the photon is detected in the final measurement, will have been successfully applied to the qubit. Then is applied as discussed above. The final measurement is then just a measurement in the polarisation basis, which can be achieved using a polarising beam splitter and photodetectors.

## Vii Conclusions

Our results provide clear guidelines for determining if the sampling is fair in any particular Bell experiment. If the goal is simply to demonstrate entanglement, rather than disprove LHV theories, then the condition required is given by Eq. (31), which can be experimentally tested. If it can be demonstrated to hold, then any violation of Bell inequalities is due to entanglement. This is relevant to quantum key distribution, where security may be proven by violation of Bell inequalities ekert (); shor (); acin (); barrett (); pironio (). In cases where there is loss, but the sampling is tested and found to be fair, then the key distribution should still be secure.

In the case where hidden variables are allowed, then the relevant condition is that the efficiency factorises as in Eq. (7). Any condition that depends on the hidden variables can not be proven to hold, because it is possible that it might be violated for values of the hidden variable that it is not possible to prepare. However, it is possible to falsify it. The great advantage of providing a necessary condition, as we have done, is that if it can be shown not to hold, then the sampling is shown to be of a form that invalidates the CHSH-Bell inequality. In contrast, if the condition that is tested is not necessary, then testing it is not useful. Showing that it does not hold does not show that the sampling is of a form that invalidates the CHSH-Bell inequality, and it cannot be conclusively shown to hold. Thus our results put testing of the sampling in Bell experiments aden () on a rigorous basis.

These results also cast light on the effort to develop ways of enhancing Bell violations using postselection, as discussed in Refs. pawlowski (); cab (). Here we have found that the condition on the loss that is necessary to prevent violation of the CHSH-Bell inequality with postselection is also sufficient to ensure that Tsirelson’s bound is not violated. Our results show that this form of sampling cannot be used to enhance violation of Bell inequalities beyond what is possible without postselection.

This suggests that is should not be possible to violate Tsirelson’s bound with postselection while retaining a valid Bell inequality (as claimed in cab ()). On the other hand, it is possible for postselection to enhance the violation of Bell inequalities up to Tsirelson’s bound without invalidating them. For example, Procrustean entanglement concentration Bennett () has been demonstrated to enhance the violation of Bell inequalitites Kwiat01 (). Because Procrustean entanglement concentration corresponds to fair sampling, this postselection does not invalidate the Bell inequalities for unentangled states, and also does not lead to violation of Tsirelson’s bound for entangled states.

Our results do not entirely rule out the possibility of violating Tsirelson’s bound while the CHSH-Bell inequality still holds for unentangled states. However, this requires examining the measurement used, rather than simply relying on the form of loss. We have found schemes that allow the Bell quantity to be as large as 3 before the CHSH-Bell inequality is violated with separable states. These schemes also allow the efficiency to be below the limit of derived by Ref. garg () before the value of