Quantum teleportation of qudits by means of generalized quasi-Bell states of light
D. B. Horoshko G. Patera M. I. Kolobov






























1,2]D. B. Horoshkocor1
[cor1]Corresponding authordmitri.horoshko@univ-lille.fr
1]G. Patera
1]M. I. Kolobov

[1]Univ. Lille, CNRS, UMR 8523 - PhLAM - Physique des Lasers Atomes et Molécules, F-59000 Lille, France
[2]B. I. Stepanov Institute of Physics, NASB, Nezavisimosti Ave. 68, Minsk 220072 Belarus


Quantum superpositions of coherent states are produced both in microwave and optical domains, and are considered realizations of the famous “Schrödinger cat” state. The recent progress shows an increase in the number of components and the number of modes involved. Our work creates a theoretical framework for treatment of multicomponent two-mode Schrödinger cat states. We consider a class of single-mode states, which are superpositions of N coherent states lying on a circle in the phase space. In this class we consider an orthonormal basis created by rotationally-invariant circular states (RICS). A two-mode extension of this basis is created by splitting a single-mode RICS on a balanced beam-splitter. We show that these states are generalizations of Bell states of two qubits to the case of N-level systems encoded into superpositions of coherent states on the circle, and we propose for them the name of generalized quasi-Bell states. We show that using a state of this class as a shared resource, one can teleport a superposition of coherent states on the circle (a qudit). Differently from some other existing protocols of quantum teleportation, the proposed protocol provides the unit fidelity for all input states of the qudit. We calculate the probability of success for this type of teleportation and show that it approaches unity for the average number of photons in one component above N^2. Thus, the teleportation protocol can be made unit-fidelity and deterministic at finite resources.



Bell states Entanglement Qudits Schrödinger cat Teleportation














§ INTRODUCTION
  

Superpositions of two coherent states of an optical mode for several decades attract attention of the scientific community as optical realizations of the famous “Schrödinger cat” state of a quantum system <cit.>. There are two classes of these states with distinct properties and generation methods: (i) “even” and “odd”  coherent states <cit.>, and (ii) the Yurke-Stoler coherent state <cit.>. The states of the first class contain either even or odd number of photons and are generated for high-Q microwave cavity field by interaction with non-resonant Rydberg atoms <cit.> or for traveling-wave optical field by photon subtraction from a squeezed state <cit.>. The states of the second class have a Poissonian distribution of photons and have been recently generated for microwave cavity field coupled to a superconducting qubit by nonlinear Kerr effect <cit.>. The states of both classes have been extensively studied as models of decoherence <cit.>, sources of quantum instabilities <cit.> and resources for quantum computation <cit.>.

Splitting these superpositions in two modes, one obtains entangled coherent states <cit.>. The states of the first class create in this way quasi-Bell states <cit.>, having the same structure as usual Bell states of two qubits, but with two non-orthogonal coherent states as basis for each mode. These states can be applied to quantum metrology <cit.>, quantum tomography <cit.> and probabilistic quantum teleportation <cit.>, which is a key element of coherent state quantum computation. While traveling-wave superpositions can be rather easily split by a beam-splitter, cavity fields require a more sophisticated technique, realized only recently for two coupled microwave cavities <cit.>.

Increasing the number N of coherent components in a single-mode superposition, one obtains “multiple component Schrödinger cats” <cit.>. The most attention has been attracted to coherent states placed equidistantly on a circle <cit.>, though other geometries are also possible <cit.>. Multicomponent extensions of the second class <cit.> are known as “Kerr states” and can be generated by the same Kerr effect as their two-component variants, as has been  demonstrated recently in the microwave domain <cit.>. Production of multicomponent states of the first class has been proposed for cavity field <cit.>, but not yet reported. These states are highly important for studying  decoherence <cit.>, and for application in quantum computation with qudits, quantum systems with the number of levels higher than two <cit.>.

Splitting multiple component Schrödinger cat states in two modes, one naturally arrives at entangled coherent states of high dimension <cit.>. The states of the first class create in this way the states which are generalizations of quasi-Bell states, and their structure has been recently analyzed in detail <cit.>. These states have been proposed for enhancing sensitivity in quantum metrology <cit.>. The states of the second class, entangled Kerr states, can be used for quantum teleportation of high dimensional systems <cit.>.

In this work we further develop the approach of Ref. <cit.> and introduce explicitly entangled states of two optical modes, which we call “generalized quasi-Bell states” (GQBS). They are “quasi-Bell” because their basis vectors are not exactly orthogonal, the term having been coined in Ref. <cit.> for the N=2 case. At higher N they generalise the quasi-Bell states to higher dimensions like generalized Bell states <cit.> do for the Bell states. GQBS create a natural basis for quantum information processing with coherent states of light. In particular, we show that the protocol of probabilistic quantum teleportation works for these states much better than for the entangled Kerr states, for which it was originally suggested <cit.>. We show that the GQBS-based protocol of quantum teleportation can provide, under certain conditions, an almost unit probability and almost unit fidelity at finite resources.



§ GENERALIZED QUASI-BELL STATES

We consider one mode of the electromagnetic field, for which we fix a set of N coherent states {|α_m⟩, m=0,1,...,N-1}, placed equidistantly on the circle of radius |α_0|, i.e., α_m=α_0 e^-i2π m/N, where α_0 is an arbitrary non-zero complex number  (see Fig.<ref>).



We are interested in coherent superpositions of these states having equal weights and linear periodic relative phase:


    |c_q⟩ =  1/N√(g̃(q))∑_m=0^N-1e^i2π mq/N|α_0 e^-i2π m/N⟩,


where g̃(q) is the discrete Fourier transform,


    g̃(k)=1/N∑_m=0^N-1g(m)e^-i2π km/N=e^-|α_0|^2∑_l=0^∞|α_0|^2(k+lN)/(k+lN)!,


of the first column of the Gram matrix G_mn=⟨α_m|α_n⟩ = g(m-n), defined as


    g(m)=exp{|α_0|^2(e^i2π m/N-1)}.


Each state of the set  {|α_m⟩, m=0,1,...,N-1} is produced from the previous one in this set by a rotation in phase space  |α_m⟩=U_N|α_m-1⟩, described by the unitary operator


    U_N = e^-i2π a^† a/N,


where a is the photon annihilation operator of the optical mode. The eigenvalues of U_N are given by e^-i2π q/N. There are only N different eigenvalues, for which we let 0≤ q ≤ N-1. The corresponding eigenstates are given by Eq.(<ref>):


    U_N|c_q⟩ = e^-i2π q/N|c_q⟩.


The last property allows us to call them rotationally-invariant circular sates (RICS). They satisfy the orthonormality condition ⟨c_q|c_r⟩ = δ_qr. Using the decomposition of a coherent state in the Fock basis, we rewrite the RICS, Eq.(<ref>), in the form <cit.>


    |c_q⟩ =  e^-|α_0|^2/2/N√(g̃(q))∑_l=0^∞α_0^q+lN/√((q+lN)!)|q+lN⟩,


where |q+lN⟩ is a Fock state with q+lN photons. Eq.(<ref>) shows that a RICS is a sum of Fock states with the number m of photons such, that (m  N)=q. In the case of N=2 this property is reduced to a fixed parity of the photon number, peculiar to “even” and “odd” coherent states. In general, RICS are highly nonclassical, their distance from the set of classical states <cit.> is lower-bounded by √(1+2⟨ n⟩)-1, where ⟨ n⟩ = ⟨c_q|a^† a|c_q⟩ is the mean photon number. Thus, with growing number of photons these states become harder to create and control. However, as we show, even for low values of the mean photon number they can be used for some protocols of quantum information processing.

The states, Eq. (<ref>) have been recently considered in the case where all coherent states are almost orthogonal <cit.>, which implies sufficiently high |α_0| and sufficiently low N. In this case they are referred to as “pseudo-number” states, while the coherent states |α_m⟩ as the corresponding “pseudo-phase” states. They create two complementary bases for an N-level system (qudit), encoded into a subspace of optical mode's Hilbert space. Note, that the second basis is non-orthogonal for low values of α_0.

Now we consider the RICS |c_q⟩ with parameters {N,√(2)α_0} at one input of a 50:50 beam-splitter with the vacuum at the other one. The state of the two output modes A and B of the beam-splitter is


    |Φ_q0⟩_AB   =   1/N√(g̃_1(q))∑_m=0^N-1e^i2π qm/N|α_m⟩_A|α_m⟩_B 
       =   ∑_k=0^N-1√(λ_k(q))|c_k⟩_A|c_q-k⟩_B,


where the second part represents a Schmidt decomposition with the Schmidt coefficients <cit.>


    λ_k(q) = g̃(k)g̃(q-k)/g̃_1(q),


and


    g̃_1(q) = ∑_k=0^N-1g̃(k)g̃(q-k) = 1/N∑_m=0^N-1g^2(m)e^-i2π qm/N,


from where the summation of the Schmidt coefficients to unity follows. Here and below all indexes and integer arguments are taken modulo N.

Now we apply the power p of the rotation operator U_N^p with 0≤ p≤ N-1 to the mode B of |Φ_q0⟩_AB and obtain the state


    |Φ_qp⟩_AB   =   1/N√(g̃_1(q))∑_m=0^N-1e^i2π qm/N|α_m⟩_A|α_m+p⟩_B 
       =   ∑_k=0^N-1√(λ_k(q)) e^-i2π(q-k)p/N|c_k⟩_A|c_q-k⟩_B,


which is, on the one hand, an extension of the quasi-Bell states <cit.> to higher dimensions, and on the other hand, an extension of generalized Bell state <cit.> to non-orthogonal basis, and which we call GQBS. Two forms of this state, presented in Eq. (<ref>), correspond to writing it in the non-orthogonal coherent basis with equal weights, or in the orthogonal RICS basis with non-equal weights.

Averaging out one mode one obtains the reduced density operator of the other one:


    ρ_A(q) = ∑_k=0^N-1λ_k(q)|c_k⟩⟨c_k|,


which tends to the completely undetermined qudit state 𝕀/N in the limit of high α_0. In this limit GQBS is maximally entangled, and its entanglement, defined as E=-{ρ_Alog_2ρ_A}, is E=log_2 N. For lower values of α_0 the reduced state, Eq. (<ref>), is not the completely undetermined one and the GQBS is non-maximally entangled. Entanglement of the state |Φ_qp⟩_AB is given in this case by the Shannon entropy of the Schmidt coefficients λ_k(q)


    E(q) = -∑_k=0^N-1λ_k(q)log_2λ_k(q),


and is a function of q (but not p). Schmidt coefficients λ_k(q) are shown in Fig. <ref> for the case where each coherent state has on average just 1 photon.



The spread of coefficients in Fig. <ref> increases with q, reaching its maximum at q=N-1. Since the entanglement is given by the Shannon entropy of the Schmidt coefficients, it is minimal at q=0 and maximal at q=N-1. The same coefficients are shown in Fig. <ref> for the case where each coherent state has on average 4 photons. The dependence of entanglement on q is more complicated in this case. The maximum is reached for q=3 and the corresponding state |Φ_3p⟩ for any p is very close to a maximally entangled state, which is reflected in its entanglement 2.97, very close to log_2N=3.






§ TELEPORTATION OF CIRCULAR STATES OF LIGHT


Quantum teleportation of optical states is a key quantum technique using an entangled state of two optical field as a resource <cit.>. Entangled two-mode states, GQBS, can be used for teleporting a superposition of states |α_m⟩ with arbitrary coefficients, known as “circular state” <cit.> and representing an optical qudit, by the protocol proposed by van Enk <cit.>. This protocol was initially devised for an entangled Kerr state as a resource, but, as we will see, it works even better for a GQBS. Since a GQBS is in general non-maximally-entangled, the teleportation has a non-unit probability of success. Below we reproduce the description of the teleportation protocol from Ref. <cit.> with a replacement of the nonlocal state.


We suppose two parties, Alice and Bob, share a GQBS |Φ_qp⟩_AB, given by Eq. (<ref>), with even number of components N=2L. Alice possesses in mode C a superposition of coherent states |α_l⟩ with arbitrary coefficients Q_l:


    |ψ⟩_C = ∑_l=0^N-1Q_l|α_l⟩_C,


that she wishes to teleport to Bob.  Alice first uses beam splitters to make L=N/2 “diluted” copies of both the state to be teleported (ending up in modes C_k for k=0,...,L-1) and of her half of the entangled state (ending up in modes A_k for k=0,...,L-1) by the process


    |α_m⟩|0⟩^⊗ L-1→ |α_m/√(L)⟩^⊗ L.


Then she applies the phase shift operator U_N^k to the mode A_k and, in order to perform her
Bell measurement, subsequently combines the modes C_k and A_k on L 50:50 beam splitters. If we call the output modes G_k and H_k for k=0,...,L-1, the resulting state is


    1/N√(g̃_1(q))∑_m=0^N-1∑_l=0^N-1e^i2π qm/NQ_l
    |α_m+p⟩_B
          ⊗_k=0^L-1|(α_l-α_m+k)/√(2L)⟩_G_k |(α_l+α_m+k)/√(2L)⟩_H_k .


Alice now performs photon-number measurements on all 2L=N output modes. She cannot find a nonzero number in every mode. But suppose she finds nonzero numbers of photons in all but one mode, say, mode H_k. Then the only terms that survive the sums over m and l in Eq. (<ref>) are those for which α_l+α_m+k = 0, that is e^-i2π l/N=-e^-i2π(m+k)/N or m+k-l=LN. The state at Bob's side reduces to


    |ψ'⟩_B = ∑_l=0^N-1e^i2π q(L+l-k)/NQ_l|α_L+l-k+p⟩_B.


Alice communicates to Bob which mode contained no photons, and Bob then applies the appropriate unitary transformation. Here, with H_k being the empty mode, he applies U_N^k-p-L to his state to obtain


    |ψ”⟩_B = e^i2π q(L-k)/N∑_l=0^N-1e^i2π ql/NQ_l|α_l⟩_B.




Since the states |α_l⟩ are non-orthogonal, the phase factor under the sum cannot in the general case be removed by a unitary transformation. It means that for exact teleportation we need to choose q=0 for the entangled state used as resource, which makes Bob's state identical to Alice's, |ψ”⟩=|ψ⟩. We see also, that the value of p does not affect the process of teleporation and is compensated at the final stage by the rotation operator, so that we can put p=0 from the beginning, and consider the state |Φ_00⟩_AB as the optimal resource for quantum teleportation. The analysis of the previous section (see also Ref. <cit.>) shows that the case of q=0 does not always correspond to maximal entanglement for given N and α_0, but employment of other GQBS for quantum teleportation is not possible if one requires an exact reproduction of the initial state. Occurrence of zero-photon measurement outcome in more than one mode leads to protocol failure, thus the described protocol is probabilistic.

The possibility of realizing an exact, although probabilistic, teleportation of an arbitrary circular state on the basis of GQBS is a serious advantage compared to the original teleportation scheme <cit.>, where the final state contains phase factors quadratic in l, which cannot be corrected by any unitary transformation.




§ PROBABILITY OF SUCCESS


Teleportation described in the previous section is probabilistic, it succeeds if a zero number of photons is found in one of the measured modes only. If zero photons is found in two or more modes, the protocol fails. The probability of success depends in general on the input state. We show first how this probability can be obtained for a coherent state at the input, and then pass to the general case.

We start with finding the probability of success for the case where the state to be teleported is one of the states |α_m⟩. Thanks to the rotational symmetry, we can choose this state as |ψ⟩_C=|α_0⟩_C without loss of generality. The shared entangled state which we consider is |Φ_00⟩_AB, the one providing an exact teleportation. For such a choice the multimode state, Eq. (<ref>), takes the form


    |Ψ⟩ = 1/N√(g̃_1(0))∑_m=0^N-1
    |α_m⟩_B ⊗_k=0^L-1|α_0-α_m+k/√(N)⟩_G_k |α_0+α_m+k/√(N)⟩_H_k .



The probability of obtaining zero photons in the mode H_k and non-zero number of photons in the other N-1 measured modes is given by the average ⟨Ψ|Γ_H_k|Ψ⟩ of the projector


    Γ_H_k = Π̅_G_0Π̅_H_0...Π̅_G_kΠ_H_k...Π̅_G_L-1Π̅_H_L-1,


where Π=|0⟩⟨0| is the projector on the vacuum, and Π̅=𝕀-|0⟩⟨0| is the projector on the non-vacuum state of the mode, whose label is indicated by the lower index. If we denote the summand in the right hand side of Eq. (<ref>) by |Ψ_m⟩, then it is easy to see that only the state |Ψ_L-k⟩ makes a non-zero input to ⟨Ψ|Γ_H_k|Ψ⟩. Indeed, each other state has vacuum in a mode different from H_k and gives zero when averaged with the projector Π̅ of this mode. Thanks to the symmetry of all N modes the total success probability is N times the probability of the successful outcome in one mode. Finally we find


    P_success   =    N⟨Ψ_L-k|Γ_H_k|Ψ_L-k⟩
       =   1/Ng̃_1(0)∏_l=1^N-1(1-e^-|α_0-α_l|^2/N).



This probability is shown in Fig. <ref> for different values of N. We see that a practical value 0.2 of probability can be reached for the case of 4 components for |α_0|≈1.15, available in the optical domain <cit.>, and for the case of 8 components for |α_0|≈3.1, available in the microwave domain <cit.>.




In a similar way we can find the success probability of the original protocol of Ref. <cit.>. Expression for this probability coincides with Eq. (<ref>) if we omit the normalisation factor before the product. However, since at |α_0|>1 we have Ng̃_1(0)≈1, which means that for practical values of the amplitude the success probability is very close to that of the protocol based on GQBS.

Now we pass to the general case of arbitrary circular state at the input of the teleportation protocol. The state of all modes before the measurement is given by Eq. (<ref>) with q=p=0, which can be rewritten as


    |Ψ⟩ = ∑_k=0^L-1(|Ψ^G_k⟩+|Ψ^H_k⟩),


where


    |Ψ^G_k⟩   =   1/N√(g̃_1(0))∑_l=0^N-1Q_l
    |α_l-k⟩_B |0⟩_G_k|2α_l/√(N)⟩_H_k
          ⊗_j  k|α_l-α_l-k+j/√(N)⟩_G_j |α_l+α_l-k+j/√(N)⟩_H_j .


is the state with the vacuum in the mode G_k, and


    |Ψ^H_k⟩   =   1/N√(g̃_1(0))∑_l=0^N-1Q_l
    |α_l-k+L⟩_B |2α_l/√(N)⟩_G_k|0⟩_H_k
          ⊗_j  k|α_l-α_l-k+j+L/√(N)⟩_G_j |α_l+α_l-k+j+L/√(N)⟩_H_j .


is the state with the vacuum in the mode H_k. The probability of obtaining zero photons in the mode H_k and non-zero number of photons in the other N-1 measured modes is given by the average ⟨Ψ|Γ_H_k|Ψ⟩ of the projector, defined by Eq. (<ref>). It is easy to see, that ⟨Ψ|Γ_H_k|Ψ⟩ = ⟨Ψ^H_k|Γ_H_k|Ψ^H_k⟩, since all other states have the vacuum state in one of the modes other than H_k, and give zero when averaged with the projector Π̅ of this mode. Similarly, we find that the probability of obtaining zero photons in the mode G_k and non-zero number of photons in the other N-1 measured modes is given by the average ⟨Ψ^G_k|Γ_G_k|Ψ^G_k⟩ of the projector Γ_G_k, defined by Eq. (<ref>) with exchanged modes G_k and H_k.

The total success probability is


    P_success = ∑_k=0^L-1(⟨Ψ^G_k|Γ_G_k|Ψ^G_k⟩ +⟨Ψ^H_k|Γ_H_k|Ψ^H_k⟩)


and can be calculated numerically from Eqs. (<ref>) and (<ref>) for any input state, defined by the choice of coefficients Q_l.

We calculate the success probability for a RICS |c_q⟩, defined by Eq. (<ref>), as an input state. For this state Q_l=N^-1g̃(q)^-1/2e^i2π ql/N. The success probability is shown in Fig. <ref> for the cases N=2 and N=4.




We see that the success probability for the teleportation of RICS tends to unity for |α_0| approaching N, as it was for a coherent state. However, its behaviour at |α_0|→0 is not always the same. The success probability tends to zero in the limit of low α_0 for all states except for q=N-1, where the probability is non-zero at whatever low amplitude. This peculiarity can be understood from Eq. (<ref>), showing that a RICS  |c_q⟩ has q photons at minimum, and exactly q photons at α_0 approaching zero. Thus, before the measurement the N modes {G_k,H_k,k=0,...,L-1} have at least q photons in total. One of these modes is always in the vacuum state due to destructive interference, therefore at least q photons are distributed in N-1 modes. When q<N-1, the probability to find at least one photon in each of N-1 modes tends to zero with the amplitude. But when q=N-1 this is not the case, since N-1 photons can be found in N-1 modes, one photon per mode, and P_success at |α_0|→0 gives the probability of this event. In particular, for N=2, q=1 we have at least one photon in one mode, which is necessarily detected (we imply the unit detection efficiency). That is why the teleportation of this particular RICS is deterministic at any amplitude, as shown in Fig. <ref>.

To conclude this section, let us compare the teleportation protocol based on GQBS to other continuous variables teleportation protocols <cit.>. The protocol based on the two-mode squeezed state as a shared resource <cit.> is deterministic, but provides a non-unit fidelity. Increase of fidelity to unity requires nonphysical amounts of squeezing and correspondingly energy for the resource state. The same problem takes place for the protocol based on quantum nondemolition interaction <cit.>, which is also deterministic, but where the unit fidelity can be reached only at an infinitely strong coupling of two optical modes. The protocol of van Enk <cit.>, based on entangled Kerr states, suffers from the same problem: it cannot provide a unit fidelity for all input states, as discussed above. On the other hand, the protocols based on multiple single-photon teleportation channels <cit.> are capable of approaching the unit fidelity at finite resources, but are essentially probabilistic, because they require distinguishing all four Bell states of two photons, which is difficult at the current level of technology. The GQBS-based teleportation protocol described above relies on linear optics and photodetectors distinguishing the absence and the presence of photons (with a close to unit quantum efficiency). This protocol is deterministic for |α_0|≥ N and provides the unit fidelity for the circular states of one optical mode, defined by Eq. (<ref>). It means that for the states of this important class, perspective for quantum information processing <cit.>, our teleportation scheme is preferable to any other scheme, proposed up to date. An interesting question arises: What happens if the described scheme is applied to an arbitrary state, non necessarily circular? Obviously, since the output state is always a circular one, it cannot coincide with the input state, thus the fidelity is never unit for a non-circular input. However, for an input state with the average photon number ⟨ n⟩, choosing N≫⟨ n⟩, as follows from Eq. (<ref>), one can approximate the input state by a superposition of RICS with arbitrary precision:


    ∑_n=0^∞r_n|n⟩≈∑_q=0^N-1r_q|c_q⟩,


where r_n are any coefficients. The state in the right hand side of Eq. (<ref>) is circular and the fidelity of its teleportation can be made arbitrarily close to unity. Thus, the described teleportation protocol has high potential for quantum information processing, since it can provide an almost unit probability and almost unit fidelity at finite resources for teleportation of optical states with a sufficiently low average photon number.




§ PSEUDO-PHASE STATE AND GENERALIZED BELL STATES


In the regime where all coherent states in the superposition can be considered mutually orthogonal the set of these states is a discrete Fourier transform of the set of RICS and vice versa. That is why RICS can be considered as pseudo-number states and the coherent states as pseudo-phase states <cit.>. Measuring the number of photons in a RICS |c_q⟩ one obtains q+lN, as shown by Eq. (<ref>), which justifies its name of pseudo-number state. A coherent state has rather well-defined phase, which justifies its name of pseudo-phase state. Both state sets are orthonormal in this regime. At lower |α_0| the set of RICS remains orthonormal, but the set of coherent states |α_k⟩ does not. Following the approach of Pegg and Barnett <cit.>, we can introduce a set of pseudo-phase states as the discrete Fourier transform of the set of the pseudo-number states:


    |φ_k⟩ =  1/√(N)∑_q=0^N-1e^-i2π qk/N |c_q⟩
    =∑_m=0^N-1δ̃_mk|α_0 e^-i2π m/N⟩,


where


    δ̃_mk =  1/N^3/2∑_q=0^N-11/√(g̃(q))e^i2π (m-k)q/N,


is an almost diagonal matrix, close to the Kroneker delta δ_mk, with which it coincides at high |α_0|, where g̃(q)→1/N. The states |φ_k⟩ are mutually orthogonal ⟨φ_k|φ_l⟩=δ_kl and create a mutually unbiased basis with RICS: |⟨φ_k|c_q⟩|=1/√(N). Using these states as basis, we can construct the true generalized Bell states <cit.> for two optical modes


    |Φ̃_qp⟩_AB   =   1/√(N)∑_m=0^N-1e^i2π qm/N |φ_m⟩_A|φ_m+p⟩_B 
       =   1/√(N)∑_k=0^N-1 e^-i2π(q-k)p/N|c_k⟩_A|c_q-k⟩_B,


which can be used for standard deterministic teleportation of qudits. However, the way of generation of the state Eq. (<ref>) is not clear, while a GQBS can be produced by beam-splitting a multicomponent cat state, as shown by Eq. (<ref>).



§ CONCLUSION

We have introduced a class of entangled states of two optical modes, GQBS, which are direct generalizations of Bell states of two qubits to the case of N-level systems encoded into superpositions of coherent states on the circle. We have shown that these states can be written in orthogonal bases where they have non-uniform coefficients. We have shown that an exact probabilistic teleportation of circular states of optical mode (optical qudits) is possible on the basis of these states and that the GQBS |Φ_00⟩_AB is the optimal resource for this purpose. The probability of teleportation success is reasonably high for currently available sizes of cat states in the optical and the microwave domains, which allows us to hope for a possible experimental realisation of the proposed teleportation protocol. We have shown that for sufficiently high coherent amplitude and number of components this teleportation protocol can approach unit fidelity and unit probability at finite resources for any input state. We have also discussed the true generalized Bell states of two optical modes and shown that they are related to nonclassical pseudo-phase states. The obtained results can be useful for various schemes of quantum metrology and quantum information processing on the basis of information encoding in superpositions of coherent states of light.




§ ACKNOWLEDGMENTS


The authors are grateful to Stephan de Bièvre for many fruitful discussions. This work was supported by the European Union's Horizon 2020 research and innovation programme under grant agreement No 665148 (QCUMbER).

















  
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