# Constructing Pauli pulse schemes for decoupling and quantum simulation

## Abstract

Dynamical decoupling is a powerful technique to suppress errors in quantum systems originating from environmental couplings or from unwanted inter-particle interactions. However, it can also be used to selectively decouple specific couplings in a quantum system. We present a simple and easy-to-use general method to construct such selective decoupling schemes on qubit and qudit networks by means of (generalized) Pauli operations. As these constructed schemes can suppress Hamiltonian interactions on general qudit networks selectively, they are well suited for purposes of approximate quantum simulation. Some examples are presented, demonstrating the use of our method and the resulting decoupling schemes.

###### pacs:

03.67.Pp,03.65.Aa## I Introduction

An important challenge in quantum information science is to protect quantum memories and communication channels against unwanted couplings within this quantum system or to an environment. It is to this end that, in 1999, Viola et al. presented a promising method they called dynamical decoupling (1). In this method, local control operations are used to counteract the influence of unwanted couplings with an environment. It can be seen as a generalization of techniques which were previously developed in the area of nuclear magnetic resonance. The spin-echo effect (2) is a well-known example of the latter. Over the years, dynamical decoupling has been successfully implemented in experimental setups to protect quantum systems against unwanted influences (3); (4); (5); (6); (7).

Typically, dynamical decoupling schemes assume that the quantum system to be protected can be manipulated by a set of fast local control operations. As a first approximation, it is often assumed that these control operations act instantaneously (bang-bang control (8)) and that they can be represented by a set of unitary operators. By choosing an appropriate set of unitary operators and applying them in a particular order, it is possible to change the state of a quantum system unitarily such that the effects of unwanted Hamiltonian interactions are averaged out approximately. In contrast to quantum error correction, which is capable of correcting errors perfectly, dynamical decoupling generally only suppresses unwanted couplings.

However, the use of unitary control operations is not limited to suppressing decoherence effects or unwanted intra-particle couplings within a many-particle quantum system. Viola et al. (9) already showed that dynamical decoupling can also be used to suppress only certain components of a many-particle Hamiltonian selectively. Thus, it is possible to develop control strategies that, within certain limits, are suitable for the purpose of quantum simulation, meaning that the effects of a present Hamiltonian interaction with active controls on a quantum system resemble those of a different Hamiltonian. Wocjan et al. (10) demonstrated that any quantum system with a non-trivial Hamiltonian can simulate any other Hamiltonian interaction, provided that a suitable finite set of unitary control operations is available. Dodd et al. (11) showed that any two-body Hamiltonian on a qubit network can be simulated by any two-body entangling Hamiltonian with the help of local unitaries, a result that was generalized to qudit systems by Nielsen et al. in (12).

For purposes of quantum information processing, it is of particular interest to develop error-suppressing dynamical decoupling schemes and quantum simulation schemes for systems comprised of distinguishable qubits. For these systems, a special case of decoupling controls is frequently discussed where all control operations consist of instantaneously applied Pauli operations acting locally on each qubit separately. Numerous efficient schemes of this kind have been developed which are capable of suppressing environmental errors or unwanted inter-qubit couplings in many-qubit systems. Stollsteimer and Mahler (13), for example, proposed a construction based on orthogonal arrays, while Leung (14) presented a decoupling method based on Hadamard matrices. Both approaches were eventually unified by Rötteler and Wocjan (15). Wocjan et al. also discussed applications of similar constructions to quantum simulation scenarios (16). Furthermore, several advanced control strategies have been devised to enhance the performance of basic decoupling schemes.

Despite these interesting developments, it remains a challenge to find and implement suitable Pauli pulse schemes for the purpose of quantum simulation. While specific constructions for specific scenarios have been developed, so far there has been no systematic method for constructing dynamical decoupling schemes from simple Pauli pulses for a general scenario that applies to both error suppression and quantum simulation for arbitrary many-body Hamiltonians.

In this paper, we present a systematic method for constructing decoupling schemes from local Pauli pulses on networks of qubits that are capable of changing the action of a given arbitrary Hamiltonian to that of a wanted ”ideal” Hamiltonian . Only (partial) knowledge of and is required; there is no dependency on the availability of, e.g., suitable orthogonal arrays. This method is not only useful for protecting specific inter-particle couplings against unwanted couplings or environmental influences, but also for simulating ideal Hamiltonian dynamics within certain limits. The restriction to local Pauli operations leads to a particularly simple, but still powerful procedure which exploits two basic properties of the Pauli operators, namely that they are Hermitian and unitary and that they fulfill characteristic Clifford-type algebraic relations. We will also show that certain aspects of these properties carry over to generalized spin operators, allowing our method to be generalized to qudit networks of arbitrary dimension. Although the method does not work for all possible pairs of and , its limitations are easily understood and still allow for a multitude of interesting applications.

The outline of this paper is as follows: In Sec. II, we briefly summarize the basics of dynamical decoupling in qubit systems which are important for our subsequent discussion. In Sec. III, a general method for designing dynamical decoupling schemes based on Pauli pulses is presented which is capable of simulating an ideal many-qubit Hamiltonian approximately by another many-qubit Hamiltonian . In this section, it is also shown under which conditions such schemes can be developed. In Sec. IV, our construction method is applied to some simple examples. Finally, in Sec. V, the generalization of this construction to qudit networks is discussed briefly. Technical details concerning these higher-dimensional generalizations are presented in three appendices. A fourth appendix contains details of numerical simulations conducted to study the effectiveness of some of our schemes.

## Ii Dynamical decoupling - basic facts

In this section, basic known principles of dynamical decoupling on networks of qubits are summarized which are important for our subsequent discussion.

We consider a quantum system consisting of qubits whose state space is described by the Hilbert space

(1) |

with the Hilbert space of an arbitrary environment. The time evolution of the whole system is governed by a Hamiltonian .

Let us assume that at the beginning of periodic time intervals of length we can apply instantaneously (bang-bang control) any of the unitary and Hermitian Pauli operators to any qubit individually. This results in unitary pulses of the form

(2) |

where is used if no control action is taken on a particular qubit. After such instantaneous control pulses the time evolution of the total system is described by the unitary operator (we assume )

(3) |

where we introduced the operators . This time evolution can also be described by an effective average Hamiltonian :

(4) |

The operator is arbitrary and can be chosen to be the identity operation. depends on , and we can do a Magnus expansion (17) to develop into a series of terms depending on increasing orders of , i.e.,

(5) |

The main goal of approximate quantum simulation by dynamical decoupling is to construct a sequence of control pulses such that, to the lowest order of the Magnus expansion , the original Hamiltonian is transformed into a wanted ideal Hamiltonian of the -qubit system which contains no couplings between the qubits and the environment and which may have modified inner couplings between the qubits. The lowest order of the Magnus expansion is given by

(6) |

We call a set of operators a decoupling scheme if they transform a Hamiltonian into to lowest order, as expressed by the decoupling condition:

(7) |

We allow for a possible scaling factor with . This factor may require a rescaling of the physical time of the simulated quantum system by . Such a quantum simulation is only approximate since, in general, the higher orders of do not vanish. However, as , for sufficiently small time delays these higher-order corrections become small.

One of the most important practical questions, which is addressed in the subsequent sections, is whether, for a specific choice of and , a decoupling scheme exists at all and how it can be constructed.

## Iii Dynamical decoupling schemes for approximate quantum simulation

In this section, a systematic method for constructing dynamical decoupling schemes on qubit networks is presented which is capable of transforming the dynamics of a given Hamiltonian into the dynamics of a wanted ideal Hamiltonian by only using Pauli pulses. This way, unwanted environmental interactions can be suppressed and an ideal Hamiltonian dynamics can be simulated approximately. An extension to a network of qudits of arbitrary dimension is presented in Sec. V.

### iii.1 Constructing decoupling schemes by solving linear sets of equations

Using the notation of Sec. II, we notice that on the Hilbert space of an -qubit network, the set of the operators,

(8) |

with the base-4 representation , forms a basis for linear operators on . Therefore, one can expand both -qubit system Hamiltonians and in this basis with coefficients and , i.e.,

(9) |

Here the arbitrary linear operators act on the Hilbert space of the environment. Furthermore, it is assumed that we are looking for a dynamical decoupling scheme which removes all possible couplings between the -qubit system and the environment. The part of the Hamiltonians and which acts on the environment only is denoted and its precise form is not important for our subsequent discussion. For the sake of convenience, let us also assume that both and are traceless so that the operator can be omitted from the expansion (III.1).

By inserting the basis expansion (III.1) into the decoupling condition of Eq. (7), we obtain the relations

(10) | ||||

(11) | ||||

(12) |

Since all of the control pulses are chosen from the set of basis operators , it follows from the basic algebraic properties of the Pauli operators that their products can also be expressed by one of the basis operators, up to a global phase, e.g. . Since this phase vanishes in , we can replace the sum over the operators in (10) by a sum over the basis operators , where we introduce natural number variables which count how often each basis operator occurs in our decoupling scheme . With this replacement, we arrive at relation (11). Since for all Pauli operators (including the identity operation) the Clifford-type relation holds, it is also true that . If we incorporate these signs into the variables of unit modulus, we finally arrive at relation (12).

Due to the linear independence of the operators in (8), their coefficients can be compared individually in Eq. (12). This comparison yields a system of, at most, linear equations for the unknown natural numbers . However, we immediately notice a restriction concerning the solvability of this linear system of equations: If for any either or , then the corresponding expansion coefficient of has to vanish, i.e., . This reflects the fact that any term not present in the originally given Hamiltonian cannot be created by our decoupling scheme in the ideal Hamiltonian . Furthermore, any operator of the original Hamiltonian which has nontrivial couplings with the environment, i.e., , can only be suppressed completely and thus cannot appear in the ideal Hamiltonian .

We obtain the following set of linear equations:

(13) | ||||

with denoting the set of indices of operators which are present in the basis expansion of the originally given Hamiltonian . We need to solve for the non-negative natural numbers as well as for and which are not all independent. This is due to the fact that, since is the total number of operators in our decoupling scheme, the relation must be fulfilled. Introducing variables , our system of equations is finally given by

(14) |

By construction, the fulfill the relation , and can be found by determining as the lowest common denominator for the rational numbers . One could also choose a larger denominator for . However, this would result in a structurally identical scheme that consists of repetitions of the shorter scheme.

### iii.2 Existence of solutions

Let us now address the question of under which conditions the system of linear equations (14) has suitable solutions.

Let us first analyze the set of all possible real-valued solutions for the quantities . The system of equations depends on the previously introduced variables of unit modulus, which can be computed from the algebraic properties of the operators and . Doing so for all pairs of our operator basis yields a square matrix with entries . For , we can calculate directly from the Pauli operators and obtain a so-called Hadamard matrix,

(15) |

Hadamard matrices have the characteristic property that their entries have the values and their rows are mutually orthogonal. Due to the way the operators are constructed as tensor products of Pauli operators, it follows that higher-order matrices can be constructed from lower-order ones by the recursive relation

(16) |

This recursive construction is similar to the well-known Sylvester construction for Hadamard matrices (18). From this construction, we can conclude by induction that is a Hadamard matrix. A connection between Hadamard matrices and quantum simulation schemes on qubit networks was already discovered in (14), albeit in a more limited context. Proofs of the stated properties of the system matrix can be found in Appendix B for the more general qudit case.

Since Hadamard matrices have full rank and we use only rows from the matrix in our system of equations, we can conclude that the system has infinitely many real-valued solutions for the variables . Now, let be the matrix resulting from the matrix by including only the rows with . Then we can express our system of equations (14) in compact vector form:

(17) |

Here, is the -dimensional vector of our variables , and is the -dimensional vector of the right-hand side of (14). In order to find the general solution of this linear system of equations, we first solve for the homogeneous part, . The linear space of these solutions has dimension . As the rows of the Hadamard matrix are orthogonal and the scalar product of any two row vectors and fulfills the relation

(18) |

we conclude that any multiple of a row of not contained in is a solution of the homogeneous equation. Therefore, the most general homogeneous solution is of the form

(19) |

A particular solution of the inhomogeneous equation can be constructed by noticing that from relation (18), one can conclude that

(20) |

This yields the particular solution

(21) |

Therefore, the most general solution of the system of equations is given by

(22) |

Starting from this result, we now need to construct a set of with non-negative integer values. Let us address the issue of non-negativity first. In order for to be non-negative the quantities must be non-negative, too. This latter requirement can be met by starting from an arbitrary solution of the system of equations . Because the first row of the Hadamard matrix is never a part of (due to the Hamiltonians being traceless), it is a solution to the homogeneous equation, and so an arbitrary multiple of this first row can always be added to . In particular, one can choose the multiple as over all entries in a given . Adding to ensures that all entries in the resulting solution are non-negative.

Starting from such a non-negative solution, the quantities will be integral if the numbers are rational. Whether such solutions exist depends entirely on the particular solution and therefore on the structure of the vector . For this purpose, it is required that all entries of are rational or that they share at most a common real multiplier so that , with denoting a rational vector. However, for practical purposes, we can relax this rather stringent condition. Even if the entries of are not rational, it is quite acceptable from a practical point of view to round these quantities to suitable rational numbers. This is possible because dynamical decoupling is already approximate in nature and the lowest order is linear in the quantities . Therefore, any error originating from rounding will affect linearly only, and we conclude that we can always find solutions suitable for decoupling from the linear system (14), at least approximately.

### iii.3 Practical considerations

The presented system of linear equations allows us to calculate solutions for the variables which determine how often each of the basis operators appears in the constructed decoupling scheme. Thus, these variables describe our decoupling scheme completely. This means that we can always find a decoupling scheme for any given original Hamiltonian provided the ideal Hamiltonian does not contain operators which are either missing in or which are coupled with the environment.

However, the linear system has infinitely many solutions, and consequently infinitely many decoupling schemes exist. Although they all simulate the Hamiltonian to lowest order, they can differ significantly in their size and choice of decoupling operators as well as the scaling constant . In general, it is not apparent from these characteristic quantities how a decoupling scheme performs in practice. While their effect on the lowest order of the average Hamiltonian is identical, the effect on higher orders can be very different. For practical purposes, it is usually preferable to find a decoupling sequence which is short (small ) and has a scaling as close to 1 as possible.

The most straightforward construction of a decoupling scheme is based on the particular solution , which can be readily calculated and then modified, as described, to yield a positive solution for the . Unfortunately, it turns out that the particular solution often produces very large decoupling schemes with large scaling factors . To improve the generated decoupling scheme, we need to exploit the freedom presented by the general homogeneous solution. Unfortunately, it is not apparent how to modify the particular solution in such a way that the resulting scheme has minimal and .

There is a way to find solutions to the linear system which are guaranteed to have minimal scaling . This is done by employing linear programming. Linear programming is a technique to optimize a linear objective function of a set of variables under certain linear equality and inequality constraints. In our case, we can use linear programming for the set of variables and minimize subject to the linear equality constraints (14), which will return a solution that is guaranteed to have minimal scaling. However, this approach does not guarantee a minimal scheme size . For small qubit systems with we found empirically that the particular solutions generated by typical linear programming solvers often produce sufficiently short decoupling schemes, which are practically usable, but in some instances we were able to manually construct shorter schemes with the same minimal scaling .

Given that the number of variables and the set of equations grow exponentially with the number of qubits , constructing solutions by any method will become increasingly difficult with growing . To find schemes for larger numbers of qubits, it is often better to calculate a solution for a smaller problem instance and then induce a scheme for the full system from the smaller solution.

## Iv Example applications

In the following, we present some basic examples of how to apply our scheme construction to specific scenarios.

### iv.1 Protecting a two-qubit interaction from environmentally induced decoherence

In this example, we consider two physically separated, distinguishable qubits and , which interact according to a time-independent interaction Hamiltonian . Furthermore, both qubits are coupled to independent environments and , which introduce decoherence and damping. See Fig. 1 for a visual depiction. The full dynamics of the system is then described by the most general Hamiltonian,

(23) |

where and are arbitrary Hermitian operators on their corresponding environments, and means the -th Pauli operator acting on the -th qubit. We ignore potential interactions within and between the environments as they are not relevant to our discussion.

Our goal is to find a decoupling scheme to turn the acting Hamiltonian into the ideal Hamiltonian . For this purpose, we have to solve the system of linear equations (12). The system matrix is known and independent of the two Hamiltonians involved. For the coefficients of the vector , which determine the inhomogeneous part of the set of equations, we find

(24) |

The particular solution to the set of equations allows us to construct the following decoupling scheme by means of the previously described procedure:

(25) |

Here, the two numbers and of each column represent an operator of our decoupling scheme. We see that the scheme consists of a total sequence of pulses. They involve free evolution (identity pulses applied three times) and a sequence in which all combinations of Pauli operators appear exactly once. The scaling constant for this decoupling scheme is . This is the minimal possible value of which can be verified by linear programming.

### iv.2 Protecting a gate implementation

Let us now consider a specific interaction Hamiltonian in the form of a two-qubit Heisenberg Hamiltonian,

(26) |

This Hamiltonian can be used to implement the entangling gate if applied over a time interval of duration (see, e.g., (19)). Entangling gates are particularly interesting in quantum information because they can create an entangled state from a separable two-qubit state.

For the interaction with the environment, let us now assume that each qubit is coupled to a harmonic oscillator as described by the Hamiltonian

(27) |

Here, , and , are the creation and annihilation operators of the two oscillators, and . characterizes the common strength of the coupling.

The general two-qubit protection scheme (25) can be used to protect this gate implementation. However, the Hamiltonian in (26) contains only three out of nine possible two-qubit basis operators and the error terms in (27) involve only four out of six possible operators. Taking these special circumstances into account, we can simplify the system of equations (12) by omitting eight equations. As a result, we find the significantly simpler dynamical decoupling scheme:

(28) |

This particular protection scheme involves only four decoupling operators and has an improved scaling factor of . This means that no rescaling of the interaction time is necessary, therefore allowing the gate to be implemented faster. Furthermore, the control operators required for the special scheme can be implemented with the help of pulses utilizing only and pulses, whereas the general scheme also requires pulses, so it should be easier to implement experimentally.

To study the effectiveness of our protection schemes, we conducted numerical simulations of the achievable state fidelity depending on the error strength and the pulse delay time . The results are very encouraging because even under the influence of strong errors, a state fidelity close to is reached with pulse delays as large as . A detailed presentation of the numerical results and a comparison between the two decoupling schemes is included in Appendix D.

### iv.3 Removing diagonal couplings in a closed -qubit chain

As another example, let us consider a closed chain of four qubits with coupling between each qubit pair, as depicted in Fig. 2. We can describe the couplings by the Hamiltonian

(29) |

Our goal is to eliminate the diagonal couplings between qubits 2 and 4 and between qubits 1 and 3. The ideal Hamiltonian without these diagonal couplings can be written as

(30) |

if we assume that the indexes wrap around, i.e., qubit 5 is just qubit 1 again. This scenario is an example of selective decoupling where we want to remove only certain parts of the given Hamiltonian.

Setting up the linear system is straight-forward. The system matrix is . Our set of basis operator indices occurring in consists of , with the numbers in base-4 notation so that a number corresponds to an operator . Finally, we set the vector , meaning that we want to keep the first four operators in and eliminate the other two.

We employ linear programming to construct a decoupling scheme for this scenario. The solution given by our linear programming solver leads to the following decoupling scheme:

(31) |

The scaling factor of this scheme is , meaning that the interaction time has to be doubled to compensate for the reduced interaction strength.

### iv.4 Modifying individual interaction strengths

As a final example, we demonstrate how to construct schemes which can modify individual coupling strengths between qubits. Consider a linear chain of four qubits with nearest-neighbor interactions which are all equally strong. The Hamiltonian describing these interactions is

(32) |

with an arbitrary coupling strength. Imagine that we would like to reduce the coupling strengths between qubits 1 and 2 and between qubits 3 and 4 by half, as depicted in Fig. 3. The resulting Hamiltonian would be

(33) |

Our system matrix is as before; the relevant operator indices in our set are with corresponding entries in the vector . This way we ensure that the couplings in the middle are kept intact, while the couplings at the outer edges are reduced.

By employing linear programming again, we find the following decoupling scheme with a scaling :

(34) |

With a slight modification to this example one can simulate the perfect state transfer Hamiltonian on a linear chain of qubits discovered by M. Christandl et al. (20) and independently by G. Nikolopoulos et al. (21).

## V Approximate quantum simulation in qudit systems

In this section, we briefly discuss how the construction of dynamical decoupling schemes for approximate quantum simulation can be generalized to qudit systems. Technical details of the necessary generalizations are presented in the appendices.

A qudit is a finite-dimensional quantum system with a -dimensional Hilbert space . Correspondingly, we replace the standard Pauli operators for qubits by a generalized set of spin operators (22),

(35) |

with and . For , these operators are equivalent to the Pauli operators up to phase factors. For arbitrary values of , these operators are still unitary but no longer Hermitian. They obey the following characteristic algebraic property as derived in Appendix A:

(36) |

For an -qudit system, the tensor products of these generalized spin operators, i.e.

(37) |

with and in base- representation, still form a complete operator basis. Therefore, the same approach as discussed in Sec. III.1 can be used to set up a linear system of equations derived from the decoupling condition to lowest order. Analogous to the steps involved in Eqs. (III.1) to (12), the Hamiltonians and can be expanded in the basis of these operators , and the variables , which denote how often each operator occurs in the decoupling scheme, can be determined from the resulting system of linear equations.

From Eq. (36), we notice that now the corresponding matrix has complex entries involving the -th unit roots , . By constructing analogously to the case of qubit systems, we note that its first row still consists of unit entries, while all other rows contain each of the unit roots equally often. In addition, all rows are linearly independent. Therefore, is now a complex-valued Hadamard matrix (23). Details of the properties of with proofs are given in Appendix B.

As our system of equations is now complex but the variables (or their replacements ) still have to be real valued, it is not immediately apparent whether a (suitable) solution still exists. A detailed analysis in Appendix C reveals that it is, indeed, still possible to find suitable solutions subject to the same conditions that apply to the qubit case. Thus we conclude that with these generalizations, our method works just as well for qudit networks.

## Vi Conclusions and outlook

We have presented a general method for constructing dynamical decoupling schemes for networks of qudit systems. This dynamical decoupling method is capable of simulating an ideal Hamiltonian of a general qudit network and of decoupling this system from unwanted environmental influences approximately. The proposed decoupling schemes involve local applications of Pauli operators or of their higher-dimensional generalizations only, so that they offer interesting perspectives for experimental applications.

We have exemplified the usage of our method in three different scenarios. Those scenarios cover typical cases for our method: decoupling a system from its environment, selectively decoupling particular interactions between qubits, and modifying individual coupling strengths. Although they were presented in separate examples, our method also allows for any combination of these cases in a single scenario.

Due to the exponential scaling with the number of qubits of the linear system used in our method and the infinitely many solutions that exist, there are some practical limitations to be aware of. Although it is straight-forward to calculate a scheme from the particular solution, these schemes are typically very large and therefore not practical. To improve the generated scheme, one can, in principle, make use of the degrees of freedom presented by the general homogeneous solution, but so far no systematic procedure is known which guarantees a shorter and superior scheme. We briefly discussed the use of linear programming as a feasible workaround to find more suitable solutions and made use of it to find some of the schemes presented in the examples.

###### Acknowledgements.

Financial support by the BMBF-project QuOReP and by CASED is acknowledged. PB acknowledges support by RVO Grant No. 68407700.## Appendix A Basic spin operator properties

We show some algebraic properties of the generalized spin operators given in Eq. (35).

The adjoints of these operators are given by

(38) |

The product of two spin operators yields

(39) |

The generalized spin operators are unitary because

(40) |

Finally, we obtain the characteristic relation

(41) |

## Appendix B Properties of the system matrix

The system matrix is a complex matrix whose entries are determined by the base operators and given in Eq. (37), according to . The adjoint of is given by

(42) | ||||

(43) |

with a scalar product of the base- representations of and . Then it follows that

(44) |

The matrix is Hermitian because

(45) |

The entries of any row vector of the system matrix sum up to zero with the only exception being the first row . This follows from the fact that for any integral power of the unit root, , it holds that . We assume that is a non-zero component of the base- representation of . Thus, we find for the sum over the row the expression

(46) |

The same result is obtained if any component of the base- representation of is non-zero. Only if does the sum not vanish. In this case, all terms in the sum are equal to and performing the sums yields the result .

As a direct consequence, we find, for the scalar product between any two row vectors and ,

(47) |

which corresponds to the sum over the row .

From Eq. (41), it follows that for any row vector , there is another row vector whose entries are the complex conjugate of the former, i.e.,

(48) |

## Appendix C Real-valued solutions of the complex system of linear equations

Consider two Hamiltonians and given by

(49) | ||||

(50) |

where is a subset of and does not contain the pair . Therefore, these Hamiltonians are traceless. We want to find real-valued solutions to the complex system of linear equations

(51) |

with being the submatrix of consisting of all the rows for . This system of equations is only solvable if, for any , the corresponding also vanishes. (Compare with the discussion in Sec. III.1.) In the following, it is therefore assumed that for any .

As the Hamiltonians and are Hermitian, we can conclude that , and , provided . Therefore, we obtain the relation

(52) |

With our knowledge of the scalar products of ’s row vectors, we can conclude that a particular solution to the linear system of equations is given by

(53) |

since . This particular solution is real-valued because for any entry of the vector , we find

(54) |

The expression in brackets in (54) is of the form so that it is real valued. Adding a solution of the homogeneous equation to yields again a solution of the linear system of Eq. (51). From the scalar products in Eq. (47), we can conclude that any row vector is a solution of the homogeneous system of equations. Therefore, the most general solution of the linear system of equations is given by

(55) |

As , this construction allows us to find at least one real-valued and non-negative solution of the form with chosen so that all entries in are non-negative. Approximating the real values by rational numbers allows us to construct a decoupling scheme from , as explained in Sec. III.2.

## Appendix D Numerical simulations for the gate

In order to demonstrate the effectiveness of our method, we have performed numerical simulations for the scenario outlined in Sec. IV.2. We assume that two qubits are initially prepared in a separable state and evolve under the influence of the Hamiltonian as given by Eqs. (26) and (27). Without environmental interaction, this state would, after a time , evolve to the quantum state under the action of the ideal Heisenberg Hamiltonian . The final state resulting from time evolution under the total Hamiltonian and under active decoupling controls can be represented in the form

(56) |

with constituting an orthonormal basis of the environmental Hilbert space. ( denotes the initially prepared ground state of the environmental harmonic oscillators.) We have taken into account that the interaction time may need to be rescaled by the factor of the decoupling scheme which is used. This result can be compared with the ideal case by means of the reduced state fidelity

(57) |

in a convenient way.

In Fig.