# One-way quantum computing with arbitrarily large time-frequency continuous-variable cluster states from a single optical parametric oscillator

One-way quantum computing is experimentally appealing because it requires only local measurements on an entangled resource called a cluster state. Record-size, but non-universal, continuous-variable cluster states were recently demonstrated separately in the time and frequency domains. We propose to combine these approaches into a scalable architecture in which a single optical parametric oscillator and simple interferometer entangle up to ( frequencies) (unlimited number of temporal modes) into a new and computationally universal continuous-variable cluster state. We introduce a generalized measurement protocol to enable improved computational performance on the new entanglement resource.

###### pacs:

03.67.Bg,42.50.Dv,42.50.Ex, 42.65.Yj## I Introduction

One-way quantum computing Raussendorf2001 () is a form of measurement-based quantum computing (MBQC) Gottesman1999 (); Jozsa2005 () and an appealing alternative to the circuit model Nielsen2000 (), which is being more widely pursued Ladd2010 (). In one-way quantum computing, the primitives of the universal gate set are pre-encoded in a “quantum substrate” that is a generic, yet precise, entangled cluster state described by a graph specifying the entanglement structure of the qubits Briegel2001 () or qumodes Zhang2006 (). Quantum computing proceeds solely from single-node measurements on the cluster graph and feedforward of the measurement results Raussendorf2001 (); Menicucci2006 ().

Quantum error correction and fault tolerance in one-way quantum computing have been theoretically proven feasible for qubit cluster states Aliferis2006 (), with thresholds comparable to those for concatenated codes ( to ), and then later improved using topological methods to thresholds slightly above the percent level Raussendorf2006 (). Fault tolerance has recently been proven for continuous-variable (CV) cluster states in terms of required levels of squeezing, the squeezing threshold being no more than 20.5 dB for a error rate Menicucci2014 (). Since the techniques used in Ref. Menicucci2014 () mirror those in Ref. Aliferis2006 (), this threshold value is conservative and can most likely be improved.

A fully fledged, scalable experimental demonstration of one-way quantum computing has yet to be achieved, as none of the proof-of-principle implementations using four photonic qubits Walther2005 (); Barz2012 () or four optical qumodes Ukai2011 () employed a scalable architecture.

Recently, one-dimensional cluster-state entanglement was demonstrated, at record sizes, over the continuous variables represented by the quantum amplitudes of the electromagnetic field, a.k.a. qumodes. This was achieved in the frequency domain Chen2014 (), with 60 simultaneously addressable entangled qumodes, and in the time domain Menicucci2011a (); Yokoyama2013 (), with sequentially addressable entangled qumodes. Solely technical issues reduced these numbers from their potential higher values of qumodes in the frequency architecture Wang2014a () and unlimited qumodes in the temporal architecture Yokoyama2013 (). Besides this scalability breakthrough, optical implementations of quantum information offer other advantages such as room temperature operation, naturally low decoherence, and significant potential for device integration Politi2009 (); Bauters2011 ().

In this paper, we show that one can create computationally universal CV cluster states by entangling, both in time and in frequency, the quantum frequency comb of EPR pairs emitted from a single optical parametric oscillator (OPO). Based on previous results Yokoyama2013 (); Chen2014 (), the lattice for this state could potentially be up to nodes in one dimension (frequency) and unlimited in the other (time bins). We then show that this state enables universal quantum computing.

This work combines the best of all previous proposals for scalable CV cluster states: It employs Gaussian states with bipartite, self-inverse graphs—which are known to be highly scalable Menicucci2008 (); Flammia2009 ()—and reduces the experimental requirements by simultaneously utilizing both frequency multiplexing Chen2014 (); Wang2014 () and temporal multiplexing Menicucci2010 (); Menicucci2011a (); Yokoyama2013 (). In addition, these architectures are known to admit more compact computation Yokoyama2013 () with more favorable noise properties Alexander2014 () when compared to approaches based on CV cluster states generated by the canonical method Menicucci2006 (); Gu2009 (). Those so-called canonical CV cluster states Menicucci2011 ()—which also admit a temporal Menicucci2010 () and a time-frequency implementation Humphreys2014a ()—are not so easily scalable in optics due to frequent use of the CV controlled-Z gate.

Our proposal, in contrast, employs macronode-based cluster states Flammia2009 () entangled into a bilayer square lattice (BSL), which has 2 qumodes per macronode (hence ‘bilayer’), instead of 4 as in previous proposals Menicucci2008 (); Flammia2009 (); Wang2014 (); Menicucci2011 (). The BSL CV cluster state admits a more versatile elementary gate set than do canonical CV cluster states Menicucci2006 (); Gu2009 (), generalizing an analogous result for single-qumode operations on the CV dual-rail quantum wire Alexander2014 ().

The structure of this Article proceeds as follows: In Sec. II we describe the BSL resource state and give an explicit experimental procedure for how to generate it. In Sec. III we discuss the experimental requirements in detail. In Sec. IV we outline the basics of our measurement protocol. In Sec. V we describe how to implement universal quantum computation on the BSL. In Sec. VI we discuss noise due to finite squeezing and we conclude in Sec. VII.

## Ii State generation

Construction of the BSL CV cluster state is illustrated in Fig. 1 and described in more detail here. A type-II OPO is pumped at two frequencies , one of each polarization ( and ). Each pump produces a number of two-mode squeezed (TMS) states Ou1992a () over the frequency comb of the OPO eigenmodes, as shown in Fig. 1(a). These states are each a Gaussian approximation to an Einstein-Podolski-Rosen (EPR) state Einstein1935 () between two frequencies that add to the corresponding pump frequency. Now, even if the pump beams are continuous wave, we still can, and will, logically assign pieces of the output beam to sequential time bins Yokoyama2013 ().

The OPO modes have linewidth and are spaced by the free spectral range . Each output frequency has a corresponding frequency index and associated macronode index Wang2014 ()

(1) |

which we will call the node index for short and is used to label qumodes sequentially (rather than by frequency) in Fig. 1(a). Indeed, phasematching two frequencies and requires , and all TMS states are generated between adjacent node indices (i.e., Wang2014 ()) in Fig. 1(a).

A polarization rotation (by a halfwave plate at rad from the horizontal principal axis of the OPO crystals), equivalent to a balanced beamsplitter for polarization qumodes, entangles these TMS states into a temporal sequence of frequency-encoded dual-rail quantum wires Chen2014 (); Wang2014 (), as shown in Fig. 1(b). A Mach-Zehnder interferometer (MZI) of path difference Glockl2004 (); Huntington2005 () separates frequencies of even and odd frequency index (and node index) into separate beams. For all odd qumodes, the polarization is then time-delayed with respect to the polarization by the interval between two consecutive time bins. The result is shown in Fig. 1(c). A final polarization rotation on the odd qumodes (another “balanced beamsplitter”) yields the BSL graph of Fig. 1(d).

A final phase delay by (not shown) on either all odd or all even frequencies converts this into a finitely squeezed CV cluster state with the same ideal graph as in panel (d). It is this state that we call the BSL CV cluster state. The fact that the BSL is a bipartite, self-inverse graph makes this possible and ensures the scalability of the scheme Menicucci2008 (); Flammia2009 (); Menicucci2011 (); Menicucci2011a (); Wang2014 (). (See the general discussion of bipartite, self-inverse graphs in Ref. Menicucci2011 ().)

## Iii Experimental Details

We now outline the basic experimental requirements for generating the BSL CV cluster state, verifying its entanglement structure, and using it for quantum information processing.

Generating the BSL CV cluster state requires a “musical score” condition—i.e., the measurement times must be compatible with resolving all qumode frequencies: , an easily fulfilled condition. In addition, the measurement times must allow one to achieve maximum squeezing—that is, they must be at least as long as the OPO cavity storage time Reynaud1987 (). This translates into , since is also half the squeezing bandwidth Walls1994 (). This condition can also be easily fulfilled in practice Yokoyama2013 () and ensures that the time bins contain maximally squeezed qumodes, to the extent permitted by the experiment’s squeezing limit (mainly determined by the intracavity losses).

Moreover, it is important to remember that as long as the undepleted pump approximation remains valid, the number of modes to be entangled has no bearing on the required pump power. To see that the undepleted-pump approximation holds for our scheme, note that a typical 100-mW pump power (i.e., photons/s for green light) and a typical OPO cavity lifetime of 20 ns together yield pump photons available for downconversion. Squeezing of 20 dB corresponds to 24.5 OPO photons per output mode (since , with ). With each pump photon downconverting into two daughter photons, even with one million output modes the total number of pump photons required is only , which is just of the total number available. Therefore, pump depletion is indeed negligible.

To verify that the BSL CV cluster state has been generated successfully, we use a balanced homodyne measurement with a two-tone local oscillator (LO), as demonstrated in our two previous works Pysher2011 (); Chen2014 (). For entanglement characterization alone, the qumodes do not need to be separated in frequency.

When using the BSL CV cluster state for quantum information processing, complete qumode separation is required. The qumode separation is straightforward in the time and polarization domains. Experimental techniques that have been honed on classical optical frequency combs Diddams2007 () can be used for the frequency domain qumode separation. Such techniques include virtually-imaged phase arrays (VIPAs), arrayed waveguide gratings (AWGs), as well as diffraction gratings and combinations thereof. After separation, the individual beams will be directed to homodyne detectors or photon counters as required by the particular algorithm Gu2009 (). In the case of homodyne detection, the local oscillators will likely need to be derived from a stable classical comb, be it a femtosecond laser or a cavity-enhanced EOM, whose beam can be overlapped with the OPO’s and subjected to the same frequency separation method. The use of integrated optics may assist in implementing this scheme to full scale.

## Iv Basics of quantum computing on the bilayer square lattice

The BSL CV cluster state is easily shown to be universal for MBQC. Simply measure on all qumodes of one (e.g., ) polarization, resulting in a CV cluster state with an ordinary square-lattice graph, which can be used with standard CV MBQC protocols Menicucci2006 (); Gu2009 (). This is shown in Fig. 2(a).

Using so-called deletion measurements (as above) to simplify the graph structure of a CV cluster state is a standard way to prove universality of a given graph Flammia2009 (); Menicucci2011a (), but it is a wasteful procedure to follow in practice since half of the graph nodes and their connectivity are lost. More precisely, this method inefficiently uses available squeezing (and therefore entanglement Braunstein2005 ()), which leads to extra noise when using these resources for quantum computing Alexander2014 (). Furthermore, lattice edges are at to the direction of increasing temporal index, meaning that either the information must flow in a zig-zag pattern or the lattice width will have to scale linearly with the length of the computation, hindering the scheme’s scalability.

Fortunately, there exists a more favorable MBQC protocol that eschews all these complications and makes better use of the structure of the BSL CV cluster state, while still using just single-site measurements. The idea is to use both layers of the graph simultaneously and in a way analogous to the conventional (single-layer) square lattice protocol, as shown in Fig. 2(b). Each lattice site, which we call a macronode Flammia2009 (), is composed of two qumodes (one of each polarization). Qumodes with even node index carry the quantum information to be processed and are therefore called wire macronodes (for ‘quantum wires’). Those with odd node index control the connectivity between the wires and are therefore called control macronodes. Input states are localized with respect to the macronode structure and are encoded within the symmetric subspace of each macronode (defined in the section below). One- and two-qumode Gaussian gates are selected by the choice of homodyne measurement angles.

To simplify the presentation, we will introduce our protocol within the context of an infinitely-squeezed BSL resource state. Any physical CV cluster state can only be finitely squeezed Menicucci2006 (); Menicucci2011 (), and this leads to introducing finite squeezing effects into the computation Alexander2014 (), which we discuss in Sec. VI.

### iv.1 Computing with macronodes

For a given macronode with node index , comprised of individual qumodes labeled and , we define the symmetric () and anti-symmetric () qumodes via

(2) |

which is mathematically equivalent to a polarization rotation into the diagonal and anti-diagonal qumode decomposition (equivalently, a 50:50 beamsplitter between the two qumodes). Input states at a particular time step will either be the output state from the previous time step or new states directly injected into the BSL via an optical switch Yokoyama2013 (). They are localized to macronodes but distributed (symmetrically) between the two physical qumodes. We further define quadrature operators (position) and (momentum) for each qumode through , which satisfy with .

Before describing our measurement protocol, we also provide some definitions for useful CV logic gates. These include an optical phase delay by ,

(3) |

and a 50:50 beamsplitter between qumodes and ,

(4) |

We also define a (nonstandard) single-qumode squeezing operation:

(5) |

where is known as the squeezing factor. This gate is just an ordinary squeezing gate with squeezing parameter , followed by a phase delay if and only if . We chose this form of the gate so that for all real , its Heisenberg action on the quadratures is and .

As is standard in MBQC, once the entangled resource state is prepared, quantum computation proceeds solely through adaptive local measurements. Here we restrict the measurements to linear combinations of the quadrature operators, which will be shown to be sufficient to implement arbitrary multi-qumode Gaussian unitaries. Experimentally, this can be performed through homodyne detection. For any given qumode, we define the rotated quadrature operators

(6) |

where the second line shows the symplectic-matrix representation of the Heisenberg action of a phase delay by Alexander2014 ().

In Fig. 3 we show alternative (and equivalent) graphical representations of the BSL CV cluster state. Recall that within each macronode the map from the physical and logical mode labels is given by Eq. 2. We can apply this map to every macronode, giving us a graph where each node now represents the symmetric or anti-symmetric mode of the enclosing macronode, as shown in Fig. 3(c). This graph reveals a simpler underlying logical structure that will provide us with a convenient framework for describing how homodyne measurements on the physical modes can implement useful gates.

Generically, due to the non-local nature of the map from physical () to logical () mode labels, local measurements on the physical modes will effectively “stitch together” the disjoint square graphs present in Fig. 3(c). For a macronode , measurement of and can be represented by the following quantum circuit:

(7) |

where denotes the input state with respect to the logical mode tensor product structure. Above, the 50:50 beamsplitter takes us from logical to physical mode labels. Rotated quadratures are measured as in Eq. 6. Such measurements on the wire macronodes connect square subgraphs with their neighbors in the horizontal direction, enabling “wire-like” transmission along the BSL. The measurements on the control macronodes connect these neighboring wires vertically.

### iv.2 Keeping square graphs disconnected

For a fixed macronode, there exists a one-parameter class of homodyne angles that do not connect the adjacent square graphs. Specifically, when , the above circuit (7) is equivalent to

(8) |

where the single-qumode rotation gates commute with the 50:50 beamsplitter because the rotation angles are the same Gabay2016 (). This in turn is equivalent to

(9) |

where all circuit elements are now local, and we take the sum and difference of the measurement outcomes. Therefore, choosing for a particular wire or control macronode will disconnect the neighboring regions of the BSL graph in the horizontal or vertical direction, respectively. By restricting all control macronode measurements in this way and including the required post processing (i.e., sum and difference of outcomes), the disjoint square graphs of Fig. 3(c) remain uncoupled by homodyne measurements with respect to the physical modes.

## V Universal gate set

The methods above allow us to apply single-qumode gates on adjacent wires without them interacting. Alternatively, relaxing the restriction on a particuar control macronode implements a two-qumode gate between the adjacent wires at that location. In this section, we elaborate on this and construct a universal gate set for quantum computation on the BSL.

### v.1 Single-qumode gates

Fig. 4(a)–(c) shows a new way to represent the BSL such that all measurements are local, but with respect to a mixture of physical () and logical () mode labels. As information propagates along the lattice in the direction of increasing time index, information will flow strictly in the horizontal direction, and there will be no interactions between neighboring wire macronodes.

The structure shown in Fig. 4(c) is identical to a collection of CV dual-rail quantum wires Menicucci2011a (); Alexander2014 (), which are resources for universal single-qumode quantum computation. Therefore, we can implement single-qumode gates on the BSL by directly implementing the macronode protocol for the CV dual-rail wire from Ref. Alexander2014 (). We briefly review it here. If the qumodes at the left-most wire site are measured in the bases and , as depicted here,

(10) |

then (up to a displacements conditioned on the measurement outcomes and neglecting the effects of finite squeezing—see Sec. VI) the overall Gaussian unitary applied to the encoded input state is Alexander2014 () , where

(11) |

with . This is the basic building block for all single- and two-qumode gates that can be implemented on the BSL.

There is an important difference between the conventional CV dual-rail wire and the BSL, however. With respect to the original BSL time-ordered node layout [see Fig. 3(a)], it is natural to consider a single measurement step as translating input states horizontally by one time step—from wire macronode to wire macronode. This corresponds to translating two sites along the CV dual-rail wire since wire macronodes are interleaved by control macronodes, as shown here:

(12) |

where the horizontal black arrows indicate the size of each measurement step. Each measurement step implements two gates [Eq. (11)], but with one important caveat: the measurements on the control macronodes have to be constrained by the condition (for control macronode ) so that that neighboring wires decouple [as in Fig. 4(c)]. Note that these constraints jointly affect nodes of separate neighboring wires, which share a control macronode.

Although these constraints do not completely specify the set of possible measurements on the control macronodes, some care has to be taken in assigning the measurement angles. For one thing, constraining all control macronode measurements to the same angle would projectively measure the encoded information (as discussed below in Sec. V.2), thereby ending the computation at that point. On the other hand, attempting to use control macronode degrees of freedom to locally implement some desired gate on a particular wire would necessarily implement a nontrivial gate on both neighboring wires. For this reason, we fix all measurements on the control macronodes and only use the measurements on the wire macronodes to implement gates.

A particularly convenient choice is to set the homodyne angles to be (for control macronode ), where the sign alternates vertically with each row of control macronodes, as shown in Fig. 5. For one physical time step (i.e., measuring one wire macronode and its neighboring control macronodes) on a wire above a row of control macronodes, this implements

(13) |

where the first gate results from measurement of the wire macronode , and the second gate results from the measurements of the two control macronodes above and below, as in Fig. 3(a). Plugging into Eq. (11), we get

(14) |

Noting that , a single measurement step on the BSL implements or , depending on whether the control macronodes below the wire are or , respectively. Two applications of these gates generate all single-qumode Gaussian unitaries (up to displacements) Yokoyama2013 (); Alexander2014 ().

As mentioned above, we have neglected a ubiquitous phase-space displacement (dependent on the measurement outcomes) and the effects of finite squeezing in our discussion above. We did this in order to present clearly the basic logic of the protocol. The details of the additional displacements and squeezing effects can be found in Sec. VI.

### v.2 Projective measurement

### v.3 Two-qumode gates

In the above, we found that (by appropriately restricting the control macronode measurements) we could treat the BSL as a collection of independent non-interacting quantum wires. This protocol can be extended to also include a two-qumode entangling gate by lifting the measurement restrictions on control macronodes that lie between neighboring wires. This corresponds to the case shown in Fig. 4(d). We parameterize the choice of measurements by the vector of homodyne angles .

We would like our two-qumode gate protocol to be compatible with single-qumode gates applied on adjacent regions of the BSL. With respect to Fig. 4(d), we allow and to be free parameters, while , corresponding to macronode 3 being a control macronode, respectively. Correspondingly, selecting homodyne angles

(15) |

implements a two-qumode gate whose form we will now derive.

Our strategy for the derivation will be to use symmetries of CV cluster states and “beamsplitter gymnastics” to reduce the evolution to a form that can be interpreted as a combination of two steps of evolution on the CV dual-rail wire Alexander2014 () interleaved with two additional beamsplitters. To this end, we call attention to Fig. 6, which shows that measurements on the original resource shown in (a) are equivalent to the same measurements on the resource shown in (e). As such, we can read off the evolution from the last subfigure, using knowledge of evolution on the CV dual-rail wire Alexander2014 ().

We summarise this procedure here, referring to Fig. 6(e). First, the leftmost wire macronodes (2 and 4) are measured, applying to the input and teleporting the output into qumodes and , respectively. Then, the 50:50 beamsplitter between those two qumodes (dotted arrow) is applied. Next, the solid-arrow beamsplitters and measurements of the control macronodes implement the gate , teleporting the output to qumodes and at the following timestep. Finally, the last dotted-arrow beamsplitter acts on this output, concluding the evolution.

Thus, up to displacements and neglecting finite-squeezing-induced noise (see Sec. VI), the total gate applied is the combination of all of these individual gates:

(16) |

where the tensor product is . This captures the most general type of two-qumode Gaussian unitary gate compatible with our framework.

Though we have the general form, it is useful to give particular measurement parameters that reduce the two-qumode gates into a simple form. It is also desirable to choose a form that is commonly included in universal gate sets, such as the CV controlled-Z () gate Gu2009 (), defined as .

While there is no valid choice of measurement parameters in that yields an exact gate, it is possible to implement one followed by phase delays that can be corrected in the next step by applying the single-qumode measurement protocol immediately after this gate. Again assuming macronode 3 is a control macronode, choosing

(17) |

reduces Eq. (16) to

(18) |

which is a tunable-strength gate followed by (known, fixed) phase delays that can be undone at the next time step. Appendix D contains the detailed derivation. Once again, we postpone discussing finite-squeezing effects and outcome-dependent displacements until Sec. VI.

### v.4 Alternative representation of two-qumode gate implementation

In the previous two subsections, we showed how measurements on the control macronodes selected between applying either a pair of single-qumode gates or a two-qumode gate on neighboring wires. Here we provide an alternative description of this mechanism that employs more fully the graphical calculus for Gaussian pure states Menicucci2011 ().

Rather than finding a graphical description of the BSL that uses a mixture of physical and logical mode labels as in Fig. 4, we can instead consider the graphical representation of the premeasurement of the control macronodes (in analogy to “wire shortening” in cluster state terminology Gu2009 ()), as shown in Fig. 7. Note that for the measurement-based implementation of Gaussian gates, cluster nodes can be measured in any order since the result is equivalent up to a final phase-space displacement Gu2009 ().

The edge weights that are changed by the measurements are functions of the homodyne angles on the control macronodes and are given below in the large-squeezing limit. We get these from the graph transformation rules Menicucci2011 () corresponding to homodyne measurements on the physical modes of the BSL and then taking the limit (we choose this limit for clarity of presentation only). The edge weights in Fig. 7 are

(19) | ||||

(20) | ||||

(21) |

After the control macronodes are measured and when , wire macronodes 2 and 4 are clearly connected by horizontal and diagonal links [see Fig. 7(b)]. Attempting to “teleport” the input states through this highly connected resource state will entangle the input states. Contrast this with the case when [see Fig. 7(c)], where the resource state is simply a pair of unconnected entangled pairs. The latter is useful for propagating input states horizontally across the lattice without entangling the inputs Alexander2014 ().

### v.5 Achieving Universal Quantum Computation

A CV controlled- gate can be applied between any two adjacent wires at any point on the BSL by locally substituting the macronode protocol with the entangling-gate protocol described in Sec. V.3. This can be done repeatedly so long as each wire is involved in at most one gate at a time. Together with vacuum input states and Weyl-Heisenberg displacement operations, these gates are universal for multimode Gaussian computation Gu2009 ().

In order to achieve universal quantum computation, we also need to include non-Gaussian resources Gu2009 (). (Sub-universal algorithms, such as state verification Yokoyama2013 (); Chen2014 (), only require homodyne detection.) In principle, it does not matter which type of resource is used Lloyd1999 (). Typical examples include photon-counting measurements supplemented with Gaussian resources to implement a cubic phase gate Gottesman2001 () or preparation and injection of non-Gaussian magic states such as photon subtracted states Wenger2004 (). We leave the detailed implementation to future work.

## Vi Displacements and finite-squeezing effects

Thus far, we have neglected both the measurement-outcome-dependent displacements and finite squeezing effects that always arise in CV MBQC Gu2009 (); Alexander2014 (). We account for them here.

Since all evolution on the BSL can be reduced to evolution on the CV dual-rail wire (plus additional beamsplitters in the case of the two-qumode gate), all we need to do to take into account the effects of the measurement outcomes and finite squeezing is to use Eq. (3.4) from Ref. Alexander2014 (), which amounts to replacing [Eq. (11)] with

(22) |

where

(23) |

is a phase-space displacement [] that depends on the homodyne angles and associated measurement outcomes (, ), and

(24) |

is a nonunitary operator that captures the effects of finite squeezing. We recover Eq. (11) in the limit of large squeezing and when all measurement outcomes are zero:

(25) |

More generally, the displacements can either be actively corrected at each step or merely accounted for using feedforward Gu2009 ().

Noise from finite squeezing is ubiquitous in all MQBC protocols using CV cluster states, but fault tolerance is still possible using quantum error correction Gottesman2001 () provided that the overall squeezing levels—which set the amount of noise introduced per gate Alexander2014 ()—are high enough Menicucci2014 (). The only known threshold result Menicucci2014 () states that no more than 20.5 dB of squeezing will be required. Squeezing levels in temporal-mode Yokoyama2013 () and frequency-mode Chen2014 () cluster-state experiments (5 dB and 3.2 dB, respectively) fall short of this, but state-of-the-art experiments in optics Eberle2010 () are within an order of magnitude (12.7 dB). The existence of a compact and scalable protocol such as the one presented here is likely to further spur on experimental and theoretical work to close this gap.

Technical note.—The astute reader will note that this presentation differs from that of Ref. Alexander2014 () in three ways. First, the -dependent squeezing term appears after the displacements in Eq. (22), while it appears before them in Eq. (3.4) of Ref. Alexander2014 (). We have modified our displacement operator (23) accordingly (Cf. Eqs. (3.8) and (3.9) in Ref. Alexander2014 ()), which allows us to group all finite-squeezing effects to the end and allows our displacement to depend only on the measurement angles and outcomes (and not on ). Second, we have written the displacement in terms of the standard quantum-optics displacement operator, which relates to the Weyl-Heisenberg displacements as , and we ignore the overall phase. Third, we have corrected a typo in Eqs. (3.8) and (3.9) in Ref. Alexander2014 (), which is that should actually be .

## Vii Conclusion

We have proposed an extremely compact and scalable method for producing—from a single OPO and simple interferometer—a continuous-variable (CV) cluster state of unprecedented size [] that is universal for quantum computation. The proposal has all the advantages of record-breaking temporal- and frequency-multiplexed schemes Yokoyama2013 (); Chen2014 () while vastly increasing the size of the lattice by utilising both types of multiplexing at once. This is the most compact and scalable proposal for CV cluster states to date, and it is implementable today using demonstrated quantum-optical technology. In addition, we have generalized the one-way model for quantum computing to utilize the generated resource for quantum computation. The result translates familiar notions of CV measurement-based quantum computing (MBQC) to the particular state proposed here, generalizing prior work based on one-dimensional, macronode-based CV cluster states Yokoyama2013 (); Alexander2014 ().

The vast majority of the existing literature on CV cluster states to date has treated canonical CV cluster states (i.e., those described in Refs. Zhang2006 (); Menicucci2006 (); Gu2009 ()) as the appropriate target for an MBQC resource state. The work presented here—as well as the entire research direction upon which it is based—shows that we should shift the focus onto CV cluster states with a macronode structure Menicucci2008 (); Flammia2009 (); Menicucci2011a (); Wang2014 (); Alexander2014 (); Yokoyama2013 (); Chen2014 (). These schemes, which are all based on bipartite, self-inverse graphs Flammia2009 (), have been demonstrated to have unprecedented scalability Yokoyama2013 (); Chen2014 () and to admit novel, flexible Alexander2016 (), and more efficient Alexander2014 () quantum-computing schemes within the MBQC paradigm.

The work presented here further underscores this point, emphasizing the importance of bipartite, self-inverse graphs and of focussing on scalable designs from the ground up when working with CV cluster states. One might hope that the optimized protocols available for these states Alexander2014 (); Alexander2016 () could be used to improve the fault-tolerance threshold for MBQC using CV cluster states Menicucci2014 (). We leave this question to future work.

Note added in proof. Recently, the state of the art in cluster state generation and optical squeezing has substantially improved. Temporal-mode one-dimensional CV cluster states have recently reached sizes of one million modes with no sign of phase drift over the course of the experiment Yoshikawa2016 (). Optical squeezing levels have also improved, with the state of the art now at 15 dB Vahlbruch2016 ().

###### Acknowledgements.

This work was supported by the U.S. National Science Foundation under grant No. PHY-1206029 (for P.W., N.S., and M.C.’s graduate stipends and O.P.’s summer salary) and by the DARPA Quiness program (for O.P.’s summer salary). R.N.A. and N.C.M. were supported by the Australian Research Council under grant No. DE120102204.## Appendix A Graphical calculus for Gaussian pure states

Any -qumode Gaussian pure state can be represented uniquely (up to phase-space displacement and overall phase) by an -node, complex-weighted, undirected graph Menicucci2011 (). This graph can be represented pictorially or, equivalently, by a corresponding complex-valued adjacency matrix

(26) |

where and are symmetric real-valued matrices, and . This object is related to the wavefunction in the following way:

(27) |

A covariance matrix for this state can be expressed in terms of the matrices in Eq. (26). First, denote the vector of position and momentum quadrature operators as

(28) |

Then Menicucci2011 (),

(29) |

which in turn allows us to give an expression for the Wigner function:

(30) |

For some Gaussian unitary , we can define to be

(31) |

is also a Gaussian pure state (by the definition of a Gaussian unitary). How is the graph (corresponding to state ) related to the original graph by the Gaussian unitary? The Heisenberg action of on is linear, which means it can be represented as Menicucci2011 ()

(32) |

where is a symplectic matrix. If we represent as

(33) |

then the corresponding graph update rule is Menicucci2011 ()

(34) |

## Appendix B Simplified graphical calculus

In general, representing all the features of requires an appropriately connected graph with all edges (including self-loops) labeled by complex-valued weights Menicucci2011 (). When representing Gaussian pure states with uniformly weighted graphs, it is convenient to employ a simplified set of rules. In the main text and wherever possible in the supplementary material, we represent Gaussian pure states using simplified graphs, as introduced in Ref. Menicucci2011a (). This allows us to represent graph edge weights by color and omit self-loops from the illustrations.

With the exception of the (omitted) self-loop weights, the edge weights are implicitly defined as , where is called the edge-weight coefficient and can be thought of as the edge weight magnitude in the infinite squeezing limit, while

(35) |

can be thought of as a rescaling factor that depends on an overall squeezing parameter for the state. In the graphs, signs of and are represented by blue and orange coloring, respectively, and is indicated within relevant figure captions. Note that in the infinite squeezing limit (), edge weight . For all graphs, all black nodes have self-loop edges with weight , where

(36) |

Technically, the simplified graphical calculus representations used in the majority of the figures of this Article are valid for both infinite- and finite-squeezing cases Menicucci2011a (). To include finite squeezing explicitly, the full graphical calculus Menicucci2011 () must be used. To do this, simply replace the simplified disjoint square graphs in Fig. 3(c) by more detailed versions with self-loops and edge weights as in Fig. 8.

We note that there is a subtlety in Fig. 1 of the main text. The state that exists at various stages (a)–(d) of the optical circuit diagram is technically not a CV cluster state, but is in fact an -graph state Menicucci2011 () that would have an edge weight of . However, at every stage of the diagram this state can be converted into a CV cluster state with edge weights as quoted and with the same simplified graphical representation Menicucci2011a () by simply applying an optical phase delay of (a.k.a. a Fourier transform Gu2009 ()) on half the qumodes (specifically, all qumodes with either even or odd frequencies). In practice, this difference is unimportant because this phase delay can be incorporated directly into the homodyne measurements acting on the final state, and in fact, the simplified graphical calculus is defined in Ref. Menicucci2011a () to represent both types of states (i.e., with or without these final Fourier transforms).

## Appendix C Beamsplitter symmetries of a pair of two-qumode CV cluster states

We use Ref. Gabay2016 () to derive the symmetries of a pair of two-qumode CV cluster states. This result is used to equate panels (d) and (e) of Fig. 6.

Each individual CV cluster state shown in Fig. 6(d) has a graph given by

(37) |

and an alternative graph representation of Menicucci2011 (); Gabay2016 ()

(38) |

A pair of such states (one between qumodes and and a separate one between qumodes and ) has the alternative graph

(39) |

with rows and columns ordered . Note that here merely indicates a matrix Kronecker product and has nothing to do with a tensor product of Hilbert spaces.

An interferometric Hamiltonian , with , generates a symmetry of the Gaussian pure state defined by if and only if Gabay2016 (). One choice (among many) for that works for is . This generates a one-parameter class of symmetry operations Gabay2016 (), one example of which is

(40) |

Since this pair of beamsplitters is a symmetry of the pair of CV cluster states, acting with alone is equivalent to acting with alone, which is exactly the symmetry employed in Fig. 6(e).

## Appendix D Derivation of the two-qumode gate

Here we derive the two-qumode gate [Eq. (18)] implemented by using the measurement settings from Eq. (17) in Eq. (16). As usual, we neglect outcome-dependent displacements and finite-squeezing effects, with discussion of these effects relegated to Sec. VI. Before we start, we define the following abbreviations of phase shifts and squeezing on two qumodes at a time:

(41) | ||||

(42) |

For the chosen measurement settings [Eq. (17)], the bottom line of Eq. (16) (measurements of wire macronodes) gives

(43) |

where the two cases on the right correspond to the top and bottom signs, respectively, and we omit subscripts on for clarity. Next, we evaluate the top line of Eq. (16) (measurements of control macronodes), which gives

(44) |

The total gate is therefore the following product of the two lines:

(45) |

Noting that , the full gate becomes

(46) |

where we have used the Bloch-Messiah decomposition Braunstein2005 () of the gate. This reduces the gate to its final form:

(47) |

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