# Entanglement and Wigner function negativity of multimode non-Gaussian states

###### Abstract

Non-Gaussian operations are essential to exploit the quantum advantages in optical continuous variable quantum information protocols. We focus on mode-selective photon addition and subtraction as experimentally promising processes to create multimode non-Gaussian states. Our approach is based on correlation functions, as is common in quantum statistical mechanics and condensed matter physics, mixed with quantum optics tools. We formulate an analytical expression of the Wigner function after subtraction or addition of a single photon, for arbitrarily many modes. It is used to demonstrate entanglement properties specific to non-Gaussian states, and also leads to a practical and elegant condition for Wigner function negativity. Finally, we analyse the potential of photon addition and subtraction for an experimentally generated multimode Gaussian state.

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## Introduction —

Even though the first commercial implementations of genuine quantum technologies are lurking around the corner Chou et al. (2010); Abend et al. (2016); Popkin (2016); Sun et al. (2016); Valivarthi et al. (2016), much remains uncertain about the optimal platform for implementing quantum functions O’Brien et al. (2009); Veldhorst et al. (2015); Mohseni et al. (2017). However, it is clear that optics will play a major role in real-world implementations of these technologies O’Brien et al. (2009). Optical setups have the major advantage O’Brien (2007) of being highly robust against decoherence, while also manifesting high clock rates.

In an all-optical setting, there are various approaches to quantum information protocols, grouped in two classes according to the way information is encoded. Setups which use a few photons, and therefore also rely on single-photon detection to finally extract information, are referred to as discrete variable (DV) approaches. On the other hand, the continuous variable (CV) regime Braunstein and van Loock (2005) resorts to the quadratures of the electromagnetic field, ultimately requiring a homodyne detection scheme Armstrong et al. (2012). The major advantage of the latter is the deterministic generation of quantum resources, e.g. entanglement between up to millions of modes Yoshikawa et al. (2016). Such multimode entangled states, however, remain Gaussian, which implies that their CV properties can be simulated using classical computational resources Bartlett et al. (2002); Rahimi-Keshari et al. (2016). Hence, if a quantum information protocol is to manifest a quantum advantage, it requires non-Gaussian operations.

Here, we focus on two specific non-Gaussian operations: photon addition and subtraction Ourjoumtsev et al. (2006); Parigi et al. (2007); Zavatta et al. (2007, 2008). In the single-mode case, these processes are described and understood in a reasonably straightforward way (see e.g. Dakna et al. (1997)). Even though multimode scenarios prove to be much more challenging Averchenko et al. (2016), mode-selective coherent photon subtraction is gradually coming within range Ra et al. (2017). In two-mode setups these states have proven their potential, e.g., in the context of entanglement distillation Ourjoumtsev et al. (2007); Kurochkin et al. (2014); Takahashi et al. (2010). However the quantum properties of general multimode photon-added and -subtracted states remain unclear.

In this letter, we present an exact and elegant expression for Wigner functions of the state obtained from the addition or subtraction of a single photon to a general multimode Gaussian state. We derive the conditions for achieving negativity in this Wigner function, which are needed for the states to potentially manifest a quantum advantage Mari and Eisert (2012). Moreover, we explain how the multiple modes in an experimental setup Cai et al. (2017) can be entangled through mode-selective coherent photon addition or subtraction. For pure states, this entanglement is inherent in the sense that it cannot be destroyed by passive linear optics.

## Optical phase space —

The modal structure of light is essential throughout this work. In classical optics, a mode is simply a normalised solution to Maxwell’s equations. Multimode light is thus a sum of electric fields with complex amplitudes, , associated with a specific mode basis . For each mode in this decomposition the real and imaginary part of the electric field are, respectively, the amplitude and phase quadratures. Thus, light comprised of modes, is described by quadratures which are represented by a vector .

The same light can be represented in different mode bases, which boils down to changing the basis of . This implies that any normalised vector can be associated with a single mode ^{1}^{1}1We introduce the notion to emphasise vectors associated with modes.. However, the fact that quadratures always come in pairs induces additional structure on our space. This is described by a matrix that connects phase to amplitude quadratures and induces a symplectic structure. For this matrix, we have that and , for all , where denotes the innerproduct in . Because of this symplectic structure, we now refer to as the optical phase space. Furthermore, the space generated by , and its symplectic partner , is itself a phase space associated with a single mode.

The optical phase space is a basic structure from classical optics which must be quantised to study problems in quantum optics. To do so, we associate a quadrature operator to every . To be compatible with different mode bases, , must hold for any and such that . In addition, they also obey the canonical commutation relations Petz (1990); Verbeure (2011):

(1) |

which are scaled to set shot-noise to one. Moreover, these quadrature operators are narrowly connected to the creation and annihilation operators, and respectively. Note that denotes the mode in which a photon will be added or subtracted. One directly sees that , relating the action of photon creation or annihilation on different quadratures of a two-dimensional phase space to different phases.

## Truncated correlations —

We use the density matrix to represent the quantum state and deduce the statistics of quadrature measurements. This letter focuses on multimode Gaussian states , with expectation values denoted by , which are de-Gaussified through the mode-selective addition or subtraction of a photon. These procedures induce new states given by

(2) |

for addition and subtraction, respectively. The latter process has already been implemented experimentally Ra et al. (2017) following the recipe of Averchenko et al. (2016). In line with these experiments, we will first assume that , such that the initial Gaussian state is not displaced. The remainder of this letter will deal with the characterisation of these quantum states. Our initial tool to do so is the truncated correlation function, recursively defined as

(3) | ||||

where we sum over the set of all possible partitions of the set . In short, the n-point truncated correlation subtracts all possible factorisations of the total correlation. Hence, the truncated correlation functions are a multimode generalisation of cumulants. These functions are the perfect tools to characterise Gaussian states, since they have the property that for all and all . On the other hand, this implies that non-Gaussian states must have non-vanishing truncated correlations of higher orders.

Through the linearity of the expectation value, we first calculate that the two-point correlation of photon-added (“”) and -subtracted (“”) states is given by

(4) |

where , with the Gaussian state’s covariance matrix. The imaginary part of is directly inherited from (1), whereas the final term in (4) is a consequence of the photon-subtraction process. A straightforward calculation identifies

(5) |

where is the projector on , such that projects on the two-dimensional phase space associated with mode . However, the two-point correlations (4) do not offer direct insight in the non-Gaussian properties of the state. Measuring higher order truncated correlations immediately shows a more refined perspective. Indeed, after some combinatorics, we obtain Walschaers et al. (2017) that, for all

(6) | |||

(7) | |||

where is the set of all pair-partitions ^{2}^{2}2A pair-partition divides the set up in pairs..
The prevalence of these correlations is immediately the first profoundly non-Gaussian characteristic of these single-photon added and subtracted multimode states.

## Wigner function —

While the truncated correlations themselves may provide good signatures of non-Gaussianity, they do not directly allow us to extract quantum features such as negativity of the Wigner function. However, they are directly connected to the Wigner function via the characteristic function for any point in phase space ^{3}^{3}3Due to the linear structure , for any and , can be defined for non-normalised .. It can be shown Verbeure (2011) that this function can be written in terms of the cumulants:

(8) |

We then combine (8) with (6) to obtain the Wigner function as the Fourier transform of , which leads to a particularly elegant expression, and the key result of this letter (see Walschaers et al. (2017) for technical details):

(9) |

where can be any point in the optical phase space. is the initial Gaussian state’s Wigner function.

## Entanglement —

With the Wigner function (9), we have the ideal tool at hand to study the quantum properties of multimode photon-added and subtracted states. First, we use it to investigate their separability under passive linear optics transformations. We will refer to a state as passively separable whenever we can find a mode basis where the state is fully separable, i.e. where the Wigner function can be written as

(10) |

with a probability distribution and a way of labelling states. The are the coordinates of the vector in the symplectic basis where the state is separable. If no such symplectic basis exists, the state can never be rendered separable by passive linear optics, and we refer to it as inherently entangled.

We approach this question, starting from the initial Gaussian state , which generally is mixed, characterised by the covariance matrix . This implies Eisert and Wolf (2007) natural decompositions of the form , with and interpreted as covariance matrices: is associated with a pure squeezed vacuum , to which we add classical Gaussian noise given by . There are many possible choices for such and , which all allow for a rewriting of the Gaussian state in the form

(11) |

where is the displacement operator. When we insert (11) in (2), we can now rewrite the photon-added or -subtracted Gaussian mixed state as a statistical mixture of photon-added or -subtracted displaced Gaussian pure states. After a cumbersome calculation invoking the commutation relations between creation, annihilation, and displacement operators, we find the following convex decomposition of the Wigner function (9):

(12) |

where

(13) |

is a classical probability distribution. Indeed, it is straightforwardly verified that it is positive and normalised. In addition, the Wigner function for a displaced photon-added (“”) or subtracted state (“”) is found to be equal to ^{4}^{4}4(14) holds for general covariance matrices, and is therefore the general Wigner function of photon addition and subtraction from a displaced Gaussian state.:

(14) | ||||

denotes the Wigner function of the squeezed vacuum state with covariance matrix . Because is the Wigner function for a pure state, passive separability follows from the existence of a mode basis where is factorised.

Since represents the initial Gaussian state multiplied by a polynomial, it can only be factorised in the basis where is factorised. The polynomial is fully governed by the vector which is contained in the two dimensional phase space associated with the addition/subtraction mode. Hence, factorises if and only if the photon is added or subtracted to one of the modes that factorises . In other words, when we consider a pure Gaussian state in the mode basis where it is separable, we can induce entanglement by subtracting (or adding) a photon in a superposition of these modes. Moreover, it is impossible to undo the induced entanglement by passive linear optics. This induced entanglement is thus of different nature than gaussian entanglement, and is potentially important for quantum information protocols.

Furthermore, because (12) is valid for every possible choice of , we obtain that the state is passively separable whenever the subtraction or addition takes place in a mode which is part of a mode basis for which the initial Gaussian state is separable. For mixed initial states, it is unclear that subtraction or addition in a mode which is not part of such a mode basis automatically leads to inherent entanglement because also convex decompositions which are not of the form (12) must be considered. Note that alternative methods exist to assess the entanglement of general CV states Shchukin and Vogel (2006); Valido et al. (2014). However, these methods are not appropriate to gain analytical understanding of a whole class of states.

To illustrate the pure state result, we resort to an entanglement measure which is easily calculated from the Wigner function, the purity of a reduced state Ozorio de
Almeida (2009). We study the entangling potential of photon subtraction and addition from a pure Gaussian state derived from an experimentally generated sixteen-mode covariance matrix Cai et al. (2017). We use the Williamson decomposition to separate into a pure multimode squeezed state and thermal noise, and ignore this thermal contribution ^{5}^{5}5Thermal contribution is smaller than as quantified by the Hilbert-Schmidt norm: .. The squeezed mode basis of is referred to as the basis of supermodes. The single photon is added or subtracted in a random superposition of supermodes, characterised by a random

In Fig. 1, we investigate the entanglement of mode to the rest of the system. We obtain the reduced state’s Wigner function (where ) by integrating out all modes but the one associated with . We then find the purity by evaluating Ozorio de Almeida (2009)

(15) |

The smaller the value the stronger the mode is entangled to the remainder of the system. However, because we consider the entanglement of a superposition of supermodes to the remainder of the system, the mode will already be entangled in the initial Gaussian state. Therefore we also evaluate the purity obtained when the initial Gaussian state is reduced to the the mode . We see in Fig. 1 that both addition and subtraction of a photon lower the purity of the reduced state, hence increasing the entanglement between the mode of subtraction/addition and the other fifteen modes, a multimode generalisation of what was observed for two modes Kurochkin et al. (2014). Importantly, it is shown that photon subtraction typically leads to lower purities and thus distills more entanglement, which is in agreement with other recent work Das et al. (2016).

## Wigner function negativity —

Entanglement alone is, however, insufficient to reach a potential quantum advantage, we also require Wigner functions which are negative for certain regions of phase space Mari and Eisert (2012). In pursuit of this goal, it is directly seen that the Wigner function (9) becomes negative if (and only if) for some values of . Because , we can derive a particularly elegant necessary and sufficient condition for the existence of negative values of the Wigner function:

(16) |

Through the combination of condition (16) with (5) we obtain a predictive tool that can be used to determine to (from) which modes a photon can be added (subtracted) to render the Wigner function negative. Note, moreover, that inequality (16) for photon addition always holds, implying that the Wigner functions of a single-photon added state is always negative.

We can now study the condition (16) for the experimental state, characterised by in the case of photon subtraction, where the Wigner function is not guaranteed to be negative. In Fig. 2 we subtract a single photon from a supermode, which only leads to negativity if the supermode is sufficiently squeezed (this is the case for merely three modes). Nevertheless, Fig. 3 shows that subtraction from a coherent superposition of supermodes has an advantage regarding the state’s negativity. For of the randomly chosen superpositions, i.e. random choices of , the Wigner function has a negative region. This underlines the potential of mode-selective photon subtraction to generate states with, both, a negative Wigner function, and inherent entanglement.

## Conclusions —

We obtained the Wigner function (9) which results from mode-selective, pure addition or subtraction of a single photon to a non-displaced Gaussian state by exploiting truncated correlations (6). We showed that subtraction and addition in a mode for which the initial Gaussian Wigner function takes the form (10), leaves the state passively separable, i.e. any entanglement can be undone by passive linear optics. For a pure state, subtraction and addition of a photon in any other modes leads to inherent entanglement. It remains an open question whether this result can be generalised to mixed states. Moreover, we used the form (9) to derive a practical witness (16) to predict whether the subtraction process induces negativity in the Wigner function (see also Figs. 2 and 3). Particularly relevant to current experimental progress is our conclusion that subtraction from a superposition of supermodes can produce inherently entangled states with non-positive Wigner functions, thus paving the road to quantum supremacy applications.

###### Acknowledgements.

## Acknowledgements —

This work is supported by the French National Research Agency projects COMB and SPOCQ, and the European Union Grant QCUMbER (no. 665148). C.F. and N.T. are members of the Institut Universitaire de France.

## References

- Chou et al. (2010) C. W. Chou, D. B. Hume, J. C. J. Koelemeij, D. J. Wineland, and T. Rosenband, Phys. Rev. Lett. 104, 070802 (2010).
- Abend et al. (2016) S. Abend, M. Gebbe, M. Gersemann, H. Ahlers, H. Müntinga, E. Giese, N. Gaaloul, C. Schubert, C. Lämmerzahl, W. Ertmer, W. P. Schleich, and E. M. Rasel, Phys. Rev. Lett. 117, 203003 (2016).
- Popkin (2016) G. Popkin, Science 354, 1090 (2016).
- Sun et al. (2016) Q.-C. Sun, Y.-L. Mao, S.-J. Chen, W. Zhang, Y.-F. Jiang, Y.-B. Zhang, W.-J. Zhang, S. Miki, T. Yamashita, H. Terai, X. Jiang, T.-Y. Chen, L.-X. You, X.-F. Chen, Z. Wang, J.-Y. Fan, Q. Zhang, and J.-W. Pan, Nat Photon 10, 671 (2016).
- Valivarthi et al. (2016) R. Valivarthi, M. l. G. Puigibert, Q. Zhou, G. H. Aguilar, V. B. Verma, F. Marsili, M. D. Shaw, S. W. Nam, D. Oblak, and W. Tittel, Nat Photon 10, 676 (2016).
- O’Brien et al. (2009) J. L. O’Brien, A. Furusawa, and J. Vučković, Nat Photon 3, 687 (2009).
- Veldhorst et al. (2015) M. Veldhorst, C. H. Yang, J. C. C. Hwang, W. Huang, J. P. Dehollain, J. T. Muhonen, S. Simmons, A. Laucht, F. E. Hudson, K. M. Itoh, A. Morello, and A. S. Dzurak, Nature 526, 410 (2015).
- Mohseni et al. (2017) M. Mohseni, P. Read, H. Neven, S. Boixo, V. Denchev, R. Babbush, A. Fowler, V. Smelyanskiy, and J. Martinis, Nature News 543, 171 (2017).
- O’Brien (2007) J. L. O’Brien, Science 318, 1567 (2007).
- Braunstein and van Loock (2005) S. L. Braunstein and P. van Loock, Rev. Mod. Phys. 77, 513 (2005).
- Armstrong et al. (2012) S. Armstrong, J.-F. Morizur, J. Janousek, B. Hage, N. Treps, P. K. Lam, and H.-A. Bachor, Nature Communications 3, 1026 (2012).
- Yoshikawa et al. (2016) J.-i. Yoshikawa, S. Yokoyama, T. Kaji, C. Sornphiphatphong, Y. Shiozawa, K. Makino, and A. Furusawa, APL Photonics 1, 060801 (2016).
- Bartlett et al. (2002) S. D. Bartlett, B. C. Sanders, S. L. Braunstein, and K. Nemoto, Phys. Rev. Lett. 88, 097904 (2002).
- Rahimi-Keshari et al. (2016) S. Rahimi-Keshari, T. C. Ralph, and C. M. Caves, Phys. Rev. X 6, 021039 (2016).
- Ourjoumtsev et al. (2006) A. Ourjoumtsev, R. Tualle-Brouri, J. Laurat, and P. Grangier, Science 312, 83 (2006).
- Parigi et al. (2007) V. Parigi, A. Zavatta, M. Kim, and M. Bellini, Science 317, 1890 (2007).
- Zavatta et al. (2007) A. Zavatta, V. Parigi, and M. Bellini, Phys. Rev. A 75, 052106 (2007).
- Zavatta et al. (2008) A. Zavatta, V. Parigi, M. S. Kim, and M. Bellini, New J. Phys. 10, 123006 (2008).
- Dakna et al. (1997) M. Dakna, T. Anhut, T. Opatrný, L. Knöll, and D.-G. Welsch, Phys. Rev. A 55, 3184 (1997).
- Averchenko et al. (2016) V. Averchenko, C. Jacquard, V. Thiel, C. Fabre, and N. Treps, New J. Phys. 18, 083042 (2016).
- Ra et al. (2017) Y.-S. Ra, C. Jacquard, A. Dufour, C. Fabre, and N. Treps, Phys. Rev. X 7, 031012 (2017).
- Ourjoumtsev et al. (2007) A. Ourjoumtsev, A. Dantan, R. Tualle-Brouri, and P. Grangier, Phys. Rev. Lett. 98, 030502 (2007).
- Kurochkin et al. (2014) Y. Kurochkin, A. S. Prasad, and A. I. Lvovsky, Phys. Rev. Lett. 112, 070402 (2014).
- Takahashi et al. (2010) H. Takahashi, J. S. Neergaard-Nielsen, M. Takeuchi, M. Takeoka, K. Hayasaka, A. Furusawa, and M. Sasaki, Nat Photon 4, 178 (2010).
- Mari and Eisert (2012) A. Mari and J. Eisert, Phys. Rev. Lett. 109, 230503 (2012).
- Cai et al. (2017) Y. Cai, J. Roslund, G. Ferrini, F. Arzani, X. Xu, C. Fabre, and N. Treps, Nat Commun 8, 15645 EP (2017).
- (27) We introduce the notion to emphasise vectors associated with modes.
- Petz (1990) D. Petz, \ORIGselectlanguageenglishAn invitation to the algebra of canonical comutation relations, Leuven notes in mathematical and theoretical physics Series A No. 2 (Leuven Univ. Press, Leuven, 1990).
- Verbeure (2011) A. Verbeure, Many-body boson systems: half a century later, Theoretical and mathematical physics (Springer, London ; New York, 2011).
- Walschaers et al. (2017) M. Walschaers, C. Fabre, V. Parigi, and N. Treps, arXiv:1708.08412 (2017).
- (31) A pair-partition divides the set up in pairs.
- (32) Due to the linear structure , for any and , can be defined for non-normalised .
- Eisert and Wolf (2007) J. Eisert and M. M. Wolf, in \ORIGselectlanguageenglishQuantum Information with Continuous Variables of Atoms and Light, edited by N. J. Cerf, G. Leuchs, and E. S. Polzik (Imperial College Press, 2007) pp. 23–42, arXiv:quant-ph/0505151.
- (34) (14) holds for general covariance matrices, and is therefore the general Wigner function of photon addition and subtraction from a displaced Gaussian state.
- Shchukin and Vogel (2006) E. Shchukin and W. Vogel, Phys. Rev. A 74, 030302 (2006).
- Valido et al. (2014) A. A. Valido, F. Levi, and F. Mintert, Phys. Rev. A 90, 052321 (2014).
- Ozorio de Almeida (2009) A. M. Ozorio de Almeida, in \ORIGselectlanguageenglishEntanglement and Decoherence, Lecture Notes in Physics No. 768, edited by A. Buchleitner, C. Viviescas, and M. Tiersch (Springer Berlin Heidelberg, 2009) pp. 157–219.
- (38) Thermal contribution is smaller than as quantified by the Hilbert-Schmidt norm: .
- Das et al. (2016) T. Das, R. Prabhu, A. Sen(De), and U. Sen, Phys. Rev. A 93, 052313 (2016).