Introduction of the one-body correlation operator in the unitary-model-operator approach
In the earlier unitary-model-operator approach (UMOA), one-body correlations have been taken into account approximately by the diagonalization of unitary-transformed Hamiltonians in the and space. With this prescription, the dependence of the harmonic-oscillator energy () on calculated observables is not negligible even at larger model spaces. In the present work, we explicitly introduce the one-body correlation operator so that it optimizes the single-particle basis states and then reduces the -dependence. For an actual demonstration, we calculate the energy and radius for the He ground state with the softened nucleon-nucleon () interactions from Argonne v18 (AV18) and chiral effective field theory (EFT) up to the next-to-next-to-next leading order (NLO). As a result, we obtain practically -free results at sufficiently large model spaces. The present results are reasonably close to those by the other ab initio calculations with the same interactions. This methodological development enables us more systematic analysis of calculation results in the UMOA. We also discuss qualitatively the origin of the -dependence on calculated observables in a somewhat simplified way.
Over the past decade, nuclear structure for medium-mass nuclei have been extensively investigated by ab inito many-body approaches such as the coupled-cluster method (CCM) Wloch:2005 (); Hagen:2007 (); Hagen:2008 (); Hagen:2010 (); Hagen:2012-1 (); Hagen:2012-2 (); Binder:2013 (); Hagen:2014 (); Binder:2015 (), in-medium similarity renormalization group (IM-SRG) approach Hergert:2013-1 (); Hergert:2013-2 (); Hergert:2014 (), and self-consistent Green’s function method Barbieri:2009 (); Cipollone:2013 (); Soma:2014 (). For instance, the reproduction of ground-state energies for oxygen isotopes is one of the most successful examples with such methods Hagen:2012-1 (); Hergert:2013-2 (); Cipollone:2013 (). This finding supports the importance of the contributions from three-body forces for exotic nuclear structure. Also, the CCM casts light on the size of atomic nucleus from the study of neutron and weak-charge distributions of the Ca nucleus Hagen:2015gr (). In addition, the IM-SRG stimulates discussion on nuclear shape deformations with such ab initio approaches Stroberg:2016jf (), which follows the extension of the method to solve the valence-space problem for open-shell nuclei Tsukiyama:2012dw (); Bogner:2014ib ().
Similarly to these methods, the unitary-model-operator approach (UMOA) Suzuki:1994 (); Fujii:2004 (); Fujii:2009 () is also applicable to the investigation for the medium-mass nuclei. The UMOA was firstly introduced by Providência and Shakin to study the effects of short-range correlations on nuclear wave functions Providencia:1964 (); Shakin:1967 (). In those studies, the correlation operator was empirically determined. After these exploratory studies, the determination of correlation operators has been established based on a Hermitian effective-interaction theory Suzuki:1986 (); Suzuki:1987 (). Applying this on many-body systems, the Okubo-Lee-Suzuki transformation is done for many-body Hamiltonians to decouple the -particle -hole () excitations. In other words, the UMOA is natural extension of the Hartree-Fock (HF) method where only the decoupling is considered Suzuki:1988 (). For actual applications of the UMOA, only the excitations have been decoupled with the state. As mentioned in our previous publications Miyagi:2014 (); Miyagi:2015 (), the results strongly depend on the harmonic-oscillator-energy , even if these are converged with respect to the size of model space. It can be an issue to obtain reliable converged results which should be free from the underlying parameters (the model-space sizes and values) and also to compare with the other ab initio results.
According to the recent CCM study Kohno:2012 (), the -dependence can be drastically reduced by considering the one-body correlations. In the present work, we follow this study and introduce the one-body correlation operator in the UMOA in addition to the two-body correlation operator included already in the former calculations. We expect that the one-body correlation operator optimizes single-particle states and controls the -dependence on calculated observables. The main purpose of this work is to demonstrate how the introduction of the one-body correlation operator in the UMOA works well and to discuss the -dependence of the ground-state energy and point-nucleon radius for the He nucleus taken as a test case.
The outline of this paper is as follows. In Sec. II, we represent the theoretical framework of the UMOA focusing on the difference between the previous and current calculation procedures. Then, we show the results of ground-state energies and point-nucleon radii for He to check how the -dependence on these observables can be removed by the implementation of the one-body correlation operator in Sec. III. We also compare the UMOA results with the other ab initio ones with the same interactions. Finally, we summarize the present work in Sec. IV.
Ii Unitary-model-operator approach
Before discussing how the decoupling works well in the UMOA, we present theoretical structure in this section. In Sec. II.1, general transformed Hamiltonians in the UMOA are introduced to help the understanding of the difference between the formulations employed in the earlier and this studies. Then, it is referred how to truncate the model space in the UMOA in Sec. II.2. Sec. II.3 describes the actual calculation procedure focusing on the difference between the formulations employed in the former and this studies. Finally, in Sec. II.4, we mention how to calculate the observables in the UMOA.
ii.1 Similarity transformation
We begin with the many-body Schrödinger equation,
with the ground-state energy eigenvalue and eigenvector . Here, the operator is a general intrinsic Hamiltonian,
with the mass number , the momentum of the th nucleon , the nucleon mass , the interaction , and the three-nucleon interaction . The center-of-mass kinetic energy can be described with the one- and two-body terms as . Then, the Hamiltonian can be rewritten as
with the one-, two-, and three-body terms, , , and , respectively.
To decouple the state with states, the similarity transformation of the original Hamiltonian can be done as
with the unitary operator and the auxiliary potential . Here, the auxiliary potential is introduced as
so as to take into account the in-medium effects. The operator is the -body auxiliary potential. So far, the auxiliary potential can be taken arbitrarily, but is determined self-consistently as discussed in the end of Sec. II.1. With the transformation (4), the original Schrödinger equation, Eq. (1), is also transformed to
with the reference state multiplied by the unitary operator as
Since the reference state is arbitrary in principle, we take as a single Slater determinant such as the particle-hole vacuum. In the UMOA, the unitary-transformation operator is defined as the product of exponential operators up to the -body terms Suzuki:1988 (),
The exponents , , , are the one-, two-, , and -body correlation operators. They are defined as
respectively. Here, is the correlation operator acting on particles labeled by . The correlation operators are anti-Hermitian and satisfy
so that the transformation operator is unitary.
Generally, the transformed Hamiltonian is expanded by the Baker-Campbell-Hausdorff (BCH) formula as found in the CCM Hagen:2014 (). It is because the BCH expansion terminates with the finite order and is actually one of the advantages in the CCM. In contrast, the BCH expansion does not terminate with the finite order in the UMOA, as the correlation operators do not commute with each other. Therefore, the UMOA employs another type of expansion known as the cluster expansion Providencia:1964 (). Following the cluster expansion, we decompose into
according to the number of interacting particles. Note that the three- and higher-body terms can be induced by the transformation, even if the initial Hamiltonian includes up to the two-body interaction. For clarification, we show the explicit expressions of the one-, two-, and -body cluster terms:
with the terms introduced as
The transformed auxiliary potentials , , in Eqs. (14) - (16) are, in principle, arbitrary, but the determinations of them are crucial in the actual calculation. In order to determine these transformed auxiliary potentials, we recall the one-body potential appeared in the HF method. In the HF calculations, the one-body potential cancels with the bubble-diagram contributions of the two-body interaction. This procedure is applied directly to the UMOA. Since the transformed Hamiltonian contains many-body transformed interactions and auxiliary potentials, the bubble-diagram contributions come from , , and , , . The conditions of the cancellation can be represented diagrammatically in Fig. 1. The analytical expressions corresponding to Fig. 1 are
for the one-body term and
for the two-body term. Here, denotes the Fermi level and is antisymmetrized and normalized -body state. The conditions of the cancellation for three- and higher-body terms are given in the same way. Thus, the matrix elements of the transformed auxiliary potentials are Suzuki:1988 (); Suzuki:1992 ()
for the one-body potential, and
for the two-body potential. Furthermore, the auxiliary potentials , , in Eqs. (17) - (II.1) are related to the transformed auxiliary potentials , , through the relevant inverse transformations Suzuki:1988 (); Suzuki:1992 (),
The essential point in the UMOA is to determine the correlation operators. These are determined so that the transformed Hamiltonian does not induce the particle-hole excitations. There are a number of studies about the correlation operators (see, for example, Refs. Shavitt:1980 (); Westhaus:1981 (); Suzuki:1982 ()). For brevity, the determination of correlation operators is given in Appendix A. Once the correlation operators are determined, one can build up the transformed Hamiltonian with Eqs. (13) - (II.1).
ii.2 Model space
In this subsection, we present the choice of the model space employed in earlier and current UMOA calculations. To obtain converged results in relatively smaller mode spaces, the two-step decoupling method has been applied in the earlier UMOA Fujii:2004 (); Fujii:2009 (). Figs. 2 and 2 schematically show how to decouple the model space in the earlier calculations. In the first-step decoupling, the initial Hamiltonian is transformed so that the model space (the shaded area in Fig. 2) and its complement are decoupled. The aim of this step is to make bare interactions can be handled without any explicit softening of input interactions. Since this decoupling is done in the huge space to take into account short-range correlations of input bare interactions, the decoupling equation is solved with the relative and center-of-mass coordinates. Thus, our model space has to be truncated to be a triangle shape in the two-body space by . Here, and are the nodal and azimuthal quantum number of the HO basis state , respectively. By employing this effective interaction through the first-step decoupling, we further decouple the excitations with the reference state, which is illustrated by the solid arrow in Fig. 2. After the second-step decoupling, we construct the transformed Hamiltonian and obtain the observables using the transformed operators as discussed in Sec. II.4.
In the first-step decoupling, the angle-average approximation is used for the Pauli exclusion operator. The investigation of this approximation, at least for finite nuclei, may not be sufficient and can cause uncontrollable uncertainties. As discussed in Refs. Schiller:1999 (); Suzuki:2000 (); Baardsen:2013 (), it was reported that there is the non-negligible difference between the results with and without the angle-average approximation in the nuclear matter calculations. Since we would like to examine the validity of the UMOA without any uncontrollable approximations, we do not employ the first-step decoupling in the present work. Alternatively, we soften input bare interactions via low-momentum or similarity renormalization group techniques. Therefore, we consider only the process for the decoupling of the and excitations on top of the reference state. Then, the choice of the model space is no longer restricted to the triangle shape. Here, we employ the simplest square model space defined by , as shown in Fig. 3. The decoupling of the and excitations is indicated by the solid arrow in Fig. 3.
ii.3 Numerical implementation
In this subsection, we discuss the numerical implementation of the UMOA with the decoupling examined in the present work. In this study, we treat only two-body interactions and do not include any three- and higher many-body ones in the initial Hamiltonian, Eqs. (2) and (3). In addition, we keep only the one- and two-body cluster terms and correlation operators. Thus, two- and many-body auxiliary potentials in Eq. (5) are dropped out and only one-body auxiliary potentials are left. Under these conditions, the flow chart of the actual computation is illustrated schematically in Fig. 4. Each step of the procedure is also listed as follows:
The calculation is performed iteratively until is satisfied. Here, and are the one-body fields obtained at the current and previous iteration steps, respectively.
By using the operator obtained in the step 1, the original two-body interaction is transformed as
By taking the normal ordering with respect to the Fermi level,
we obtain new .
Applying the inverse transformation,
we get to be substituted into the one-body Schrödinger equation in the step 1.
After the calculation procedure described above, the correlation operators and are evaluated. Using and , we can construct the transformed Hamiltonian and then obtain the ground-state energy and wave function. Moreover, we can obtain the other expectation values of observables with the same transformed operators as discussed in Sec. II.4. This is one of the advantages about effective operators in the UMOA.
ii.4 Ground-state energy and radius
Here, we present how to calculate the ground-state energy and root-mean square radius in the UMOA. After the transformation discussed in Sec. II.3, we construct the transformed Hamiltonian up to the two-body parts with Eqs. (14), (15), (17), (18), and (29). Fig. 5 shows the schematic representations of the transformed Hamiltonians with and without the one-body correlation operator. In the previous publications Miyagi:2014 (); Miyagi:2015 (), we have employed the Hamiltonian without the decoupling () as shown schematically in Fig. 5 to evaluate the ground-state energy and radius. Instead, we diagonalized the transformed Hamiltonian in the and space to take into account the effect of off-diagonal components between the and states. While, in the present formulation, the matrix elements between the and states vanish from the beginning, because of the decoupling by the one-body correlation operator as shown in Fig 5. The ground-state energy is dictated with the transformed Hamiltonian and reference state as
The rightmost term in Eq. (31) corresponds to the zero-body term after taking the normal ordering with respect to the reference state . It is approximated up to the third order of expansion as
where is the one-body transformed kinetic energy term. The three-body cluster term is evaluated a posteriori as
One of the advantages in the UMOA is the usage of the same transformed operators for energies to obtain the other observables. Although, in principle, one can also use the transformed operator in the CCM, one has to solve the coupled-cluster equation for both of left and right eigenvectors to construct the transformation operator due to the non-Hermiticity. In practical applications, the Hellmann-Feynman theorem is often applied to obtain the observables other than energies, as found in the recent studies (see e.g., Ref Hagen:2014 ()). On the other hand, the calculation of observables is rather simple in the UMOA. For an explicit demonstration, we show how to calculate the radius in the following. Let be the squared point-nucleon radius operator defined as
with the coordinate vector of -th nucleon and of the center-of-mass . Similarly to the evaluation of ground-state energy, the squared radius operator is decomposed into the one- and two-body operators,
where and are the one- and two-body parts, respectively, as
With the aid of the unitary operator , the expectation value can be expressed by the transformed operator and the reference state as
with the transformed radius operator
Then, we carry out the cluster expansion of the transformed operator ,
Here, the one- and two-body cluster terms are generated as
The expectation value is equal to the normal-ordered zero-body term,
Here, and are the contributions of one- and two-body transformed radius operators, respectively. In actual calculations, we truncate the cluster expansion up to the second order to evaluate the radius as in Eq. (45).
Iii Results and discussion
In the earlier UMOA studies, the ground-state properties of O, Ca, and Ni have been mainly discussed with realistic interactions Suzuki:1994 (); Fujii:2004 (); Fujii:2009 (); Miyagi:2015 (); Miyagi:2014 (). Only the decoupling of the excitations has been considered, i.e., in Eq. (8). The calculated results, especially for radii, strongly depend on the values and are difficult to judge the reliability from ab-initio point of view. Following the success to reduce the -dependence in the CCM Kohno:2012 (), we naturally extend the formalism and introduce the one-body correlation operator to the UMOA in the present study. As the validation of the effectiveness, we show the numerical results of ground-state energy and point-nucleon radius of He with the transformation . Then, we discuss the role of the one-body correlation operator in the UMOA to some extent.
The choice of the initial Hamiltonian for numerical calculations is one of the important issues. Nowadays, the sophisticated nucleon-nucleon () interactions have been developed and reproduce the scattering phase shift data with the high precision, as well as the deuteron properties such as the AV18 Wiringa:1995 (), CD-Bonn Machleidt:2001 (), and chiral EFT NLO interactions Entem:2003 (). It is, however, difficult to apply directly such bare interactions to our calculations, because of the strong coupling between low- and high-momentum regions. To get rid of this computational difficulty, we have applied on the earlier UMOA the effective interactions derived with some approximations which hamper reliable estimations of the uncertainty on calculated results (see e.g. Refs. Suzuki:1994 (); Fujii:2004 ()).
In the present work, we are interested in confirming the applicability of the UMOA through the comparison to the other ab initio results. It is preferable to reduce the uncertainties coming from the effective interactions employed in the earlier UMOA as much as possible. Therefore, we omit such process in the earlier UMOA by using sophisticated softened interactions. For this purpose, we mainly use two types of interactions. One is the low-momentum interaction derived from the AV18 interaction Wiringa:1995 () with the sharp cutoff fm. The other is the SRG-transformed chiral EFT NLO interaction Entem:2003 () with the cutoff fm to compare with the recent ab initio calculation results Nogga:2004 (); Hagen:2007 (); Roth:2011 (). As the qualitative aspect between these two interactions is similar enough to discuss the role of in the UMOA, we mainly show the results with the low-momentum interaction in the following discussion. Note that our results are not comparable directly to the experimental data due to the missing genuine three-body and induced many-body interactions which cannot be treated in the formalism. We can, however, compare our present UMOA results with the other ab initio ones obtained by using the same interactions.
iii.1 Role of the one-body correlation operator
Before discussing the importance of one-body correlations in the UMOA, Fig. 6 summarizes the dependence of the model-space size on the energy and point-nucleon radius of the He ground state in the former and current UMOA. In the left panels, one-body correlations are approximately taken into account through the diagonalization in the and space as done in earlier works Fujii:2004 (); Fujii:2009 (); Miyagi:2014 (); Miyagi:2015 (). While, in the right panels, one-body correlations are explicitly included by the one-body correlation operator as in the present formalism. As seen in the figure, the convergence with respect to the size of the model space can be almost achieved around both in the earlier (in the left panels) and current (in the right panels) formulations. Interestingly, in the earlier formalism (shown in the left panels), we can observe the artificial -dependence even after the convergence for the model-space size is achieved. It is our motivation behind the employment of the one-body correlation operator in the UMOA so as to eliminate this artificial dependence. On the other hand, in the current formalism (shown in the right panels), the results show typical behavior for the and parameters found in usual ab initio calculations, i.e., the -dependence reduces as the model-space size increases. Now we can obtain the converged results by the UMOA calculations with sufficiently large model space differently than before. In the figure, the FY Nogga:2004 () and CCSD Hagen:2007 () results for the ground-state energy with the same interaction are also shown for a comparison purpose.
After confirming the convergence of the results with respect to the parameters, and , Fig. 7 compares the ground-state energies (upper panel) and point-nucleon root-mean-square radii (lower panel) of He as functions of in the earlier and current UMOA formalisms with and without the one-body correlation operator . Note that we show the results only in , because the calculated results almost converge at as found in Fig. 6. For example, the difference between our results for energies at and is order of 10 keV. It is sufficient for the present purpose of discussion. In the figure, the results without the one-body correlation operator (blue triangles) are almost parallel with the HO results (black dashed line) both for the ground-state energies and point-nucleon radii. It implies that the operator does not change the trend of the -dependence originated from the HO reference state. After the diagonalization in the and space (green squares) as employed in the earlier framework Fujii:2004 (); Fujii:2009 (); Miyagi:2014 (); Miyagi:2015 (), the -dependence on the results is slightly reduced compared to the UMOA without (blue triangles). In contrast, the situation drastically changes, if the transformation operator is constructed by the one- and two-body correlation operators as in the current formalism. The results from the UMOA with (red circles) are practically -independent both for the energy and radius. This is the main result in this paper showing that the one-body correlation operator functions well in the UMOA to reduce the -dependence, which is needed to obtain reliable converged results. In the present framework, we do not have to care about the choice of , if the calculations are done in sufficiently large model spaces.
There are additional remarks on the optimum value in the UMOA. In the CCM Kohno:2012 (), the choice of the values is discussed by comparing the results with and without the one-body correlation operator. In Ref. Kohno:2012 (), the authors concluded that the results (calculated without the one-body correlation operator) at minimizing the ground-state energy agree with the -independent results (calculated with the one-body correlation operator). This statement is confirmed by the present UMOA calculations. Our results for energies with (circles) and without (triangles) the operator are very close to each other around the optimum value of MeV in Fig 7. There is, however, a word of caution about the choice of the value for the results after the diagonalization in the earlier UMOA. In our previous investigations Miyagi:2014 (); Miyagi:2015 (), the ground-state energies and charge radii of doubly magic nuclei have been calculated in the UMOA without . Then, the results converge with respect to the model-space size, while the -dependence of the results, especially for charge radii, is not negligible. To determine accurately the radii, we have taken the results after the diagonalization at minimizing the ground-state energy, corresponding to the square symbol at MeV in Fig. 7. Since we do not confirm the agreement of the results with the diagonalization (squares) and with (circles) at MeV in Fig. 7, such an estimation would not be valid after the diagonalization. In the present framework, however, we do not have to care about the choice of , because of the weak -dependence of the results.
After glancing over the effect of the one-body correlation operator, we next discuss how the -dependence of the results is reduced by introducing the operator. To look closer the role of the one-body correlation operator, it is convenient to decompose the expectation value into the contributions from each cluster term. In the case of the ground-state energy, it can be decomposed into energies from the one-body kinetic term , two-body cluster term , and three-body cluster term . Fig. 8 describes the energies from each decomposed cluster term. The total, one-body, two-body, and three-body energies of the He ground state are shown as functions of from the top to the bottom in the figure. As a reference, the HO (dashed line) and HF (dotted) reference states are also drawn. From the figure, one can find that the contribution from the three-body cluster term is smaller by two orders of magnitude than the one- and two-body cluster terms. The cluster expansion in the UMOA converges in the case of the He ground-state energy. Also the -dependence of the energy expectation values is reduced at each order of the cluster expansion.
Now, let us focus on the one-body kinetic energy part (the second panel from the top in Fig. 8). When we ignore from the beginning (), is nothing but the sum of the diagonal component of the matrix . Here, means the expectation value of an operator with respect to the HO reference state . In the case of the He ground state, one can easily find that (denoted by the blue triangles in the second panel from the top in Fig. 8) is proportional to as
with respect to the HO reference state (0s1/2). On the other hand, when is introduced, the off-diagonal component of the original matrix contributes to . As a result, becomes practically -independent (as denoted by the red circles in the figure). Also, these are quite close to the HF kinetic energy (black dotted curve in the figure). Thus, the operator acts as the generator of the transformation from to in the UMOA.
Almost the same discussion can be done for the expectation value of the two-body cluster term. The dashed line in the third panel from the top in Fig. 8 corresponds to
which is the sum of the diagonal components of the original two-body matrix elements. As seen in the figure, it shows the monotonic dependence on . This tendency can be understood by assuming a simple -wave two-nucleon potential model such as the contact interaction regularized by the Gaussian with a cutoff momentum :
Here, and are the magnitudes of relative momenta for the initial and final states, respectively. The and are the low-energy constants for and channels, respectively. Note that only the -wave potentials are enough for the discussion about the single-particle configuration. As discussed in Appendix C, one can obtain
The -dependence is given by the derivative of with respect to . As shown in Eq. (79), the derivative is always negative in our range from 20 to 40 MeV. While the HF result (dotted curve) shows rather weaker -dependence. Similar behavior can be found in the UMOA with and without (circles and triangles, respectively). Accordingly, the -dependence is reduced by the effect of .
Similarly to the one- and two-body cluster terms, the -dependence on the three-body cluster term is also reduced as shown in the bottom panel of Fig. 8. From these considerations, the inclusion of the operator mitigates considerably the -dependence of the energy expectation value at each order of the cluster expansion. Moreover, the relations between the UMOA with and without resemble those between the results with the HF and HO states. Note that, if we ignore from the beginning, calculated ground-state energies numerically coincide with the HF ground-state energies within a few keV level. Thus, a constant shift in the two-body energy comes from the contribution.
To examine more directly the role of , the overlap of wave functions is also investigated. In Fig. 9, we show three squared overlaps obtained with the HF and HO reference states (black dashed line), the UMOA with and without (blue triangles), and the UMOA with and HF states (red circles). Note that the UMOA results are obtained at . The squared overlap (dashed line) indicates the effect of the optimization of single-particle basis states. In Fig. 9, the squared overlaps (black dashed line) and (blue triangles) behave in a similar way. Therefore, the role of is to optimize the single-particle basis states, as expected from the above discussion of the ground-state energy. As a check, we confirm that the overlap (red circles) does not depend on the values.
Further insight can be acquired by looking into the one-body density matrix . The derivation of the one-body density matrix in the UMOA is shown in Appendix B. Using Eq. (68), we have at the leading order of cluster expansion. Fig. 10 shows the density matrices for the orbital with the values ranging from 20 to 36 MeV at . For visibility of the figure, we only show the density matrices up to the components of max(, ) . When the one-body correlation operator is switched off (), only the component of the density matrix is dominant. Then, as shown in Eq. (46), linearly increases as a function of . In contrast, the off-diagonal elements, especially , can have large values, when the one-body correlation operator is turned on (). At MeV, is positive and increases . Note that the off-diagonal component of is always positive. On the other hand, is negative and decreases at MeV. The contribution from the off-diagonal components to balances around MeV, because is almost zero there. This finding is consistent with the behavior of one-body energies shown in Fig. 8.
Next, we discuss the effects of the one-body correlation operator on the point-nucleon radius. Since the radius operator is dominated by the one-body term, the one-body density matrix concerns more directly the reduction of the -dependence rather than the ground-state energy where the two-body correlations are dominant. As shown in the lower panel in Fig. 7, the point-nucleon radius of the He nucleus with respect to the HO reference state (0s1/2) can read
From the observation that the off-diagonal components of the kinetic and radius one-body operators contribute oppositely, we can expect that the radius decreases (increases) in smaller (larger) region across MeV compared to the HO reference state Eq. (50). This is consistent with the radii shown in the lower panel of Fig. 7.
iii.2 Comparison with the other ab initio results
|CCSD Hagen:2007 ()|
|FY Nogga:2004 (); Hagen:2007 ()|
|IT-NCSM Roth:2011 ()|
After discussing the introduction of the one-body correlation operator in the UMOA works well, in this section, we compare the present results with those from the other ab inito calculations. For this purpose, we employ the potential derived from AV18 two-nucleon interaction at fm throughout the comparison. In addition, we also employ the SRG transformed chiral NLO interaction Entem:2003 () with the momentum cutoff fm, which is widely used in recent ab initio calculations.
The results of the He ground-state energy are summarized in Table 1 with the comparison to the other ab inito results. In Table 1, the calculated energies are shown with the decomposition of the one-body cluster (kinetic) term, , two-body cluster (interaction) term, , the three-body cluster term, , and the total energy, for He, respectively (see Eq. (33)). All the results are calculated at and MeV. For comparison, the results by the CCSD, FY, importance-truncated no-core shell model (IT-NCSM), and experiment are taken from Refs. Hagen:2007 (), Nogga:2004 (); Hagen:2007 (), Roth:2011 (), and Wang:2012 (), respectively. We notice that the convergence with respect to the model-space size is confirmed. The difference between and results is less than the order of 10 keV both for the and SRG transformed interactions. As shown in Table 1, the contribution of the three-body cluster term, , is much smaller than that of one- and two-body cluster terms, and , respectively. Therefore, our result for the energy practically converges with respect to the cluster expansion. Moreover, the present result for the total energy, , is reasonably close to the other ab initio calculation energies. The difference between them is comparable to the size of . In other words, the contributions of the truncated cluster terms can be approximated by the size of and the uncertainty of our energies can be roughly estimated from . In Fig. 11, we also summarize the comparison of various calculated energies. The error bands of the UMOA energies are estimated from the size of the three-body cluster term corrections.
Our results for point-nucleon radius of He are listed in Table 2. It summarizes the calculated point-nucleon radii with the ”one-body cluster term ” , ”two-body cluster term” , and the ”one- and two-body cluster term” , respectively (see Eq. (45)). Caution that , and . The calculation set up is same as in Table 1. The experimental value is take from Ref. Alkhazov:1997 (). According to Table 2, the contribution from the one-body cluster term, , is dominant. Since the effects of the higher-body cluster terms can be expected to be smaller than that of one-body cluster term, the cluster expansion works well for the radius operator same as the case of the ground-state energy. Moreover, the present result for point-proton radius, 1.41 fm, with the SRG softened NLO chiral EFT interaction Entem:2003 () with fm is consistent with the in-medium SRG results with the same interaction Hergert:2016 (). Note that the calculated radius is much smaller than the experimental radius 1.49 fm. This observation is also true for the other ab initio calculations with interactions only, and is consistent with the fact of the obtained larger binding energy compared to the experimental binding energy. From these demonstrations, we can conclude that the UMOA with the aid of the one-body correlation operator gives fully-microscopic results as well as the other ab initio approaches at least in the ground-state properties of the He nucleus.
We extend the former formalism of the UMOA accommodating only two-body correlations by including additionally the one-body correlation operator. As a demonstration, we have carried out numerical calculations of the ground-state energy and point-nucleon radius for the He nucleus. We can successfully reduce the -dependence on calculated observables which exists in the earlier UMOA. The present results for converged ground-state energy and radius are reasonably close to the results from the other ab initio calculations with the same interactions. We find that the hierarchy of the cluster expansion is preserved and the -dependence can be removed order by order of the cluster expansion. The decoupling of the excitations from the reference state is related to the HF mean-field to absorb the -dependence. The origin of the -dependence in the former UMOA has also been discussed qualitatively. Concerning the behavior of the total energy as a function of , the one-body kinetic term totally entails the positive slope, while the two-body potential term causes the negative slope, which results in the parabolic shape of the total energy. The above discussion about the one-body kinetic energy can also explain the negative slope of the radius as a function of .
In this study, we only employ two-nucleon interactions without genuine and/or induced three-nucleon interactions. For quantitative comparison with experimental data, the introduction of three-body forces is requisite. For this purpose, the systematic improvement of the UMOA is necessary. The next step to be done for this direction is to explicitly deal with the three-body cluster term and to introduce the three-body correlation operator. These implementations in the UMOA described above will open the way towards fully-microscopic description of nuclear structure consistent with the other ab-inito methods. As for the physical application, in this paper, we only focus on the ground-state property of the lightest doubly-closed nucleus, He, as a test case of the implementation of the one-body correlation operator in the UMOA. Application to heavier nuclei such as O and Ca is also interested. The extension to the excited states can also be done, for example, with the method introduced in Ref. Fujii:2004 (). Furthermore, the UMOA can be applied on the nuclear structure of open-shell nuclei and gives information about the one-nucleon separation energy Fujii:2004 (); Fujii:2009 (). These studies are now on-going, and the results will be reported elsewhere in future publications.
Acknowledgements.The authors thank M. Kohno, K. Suzuki, H. Kumagai, S. Fujii, N. Shimizu, B. R. Barrett, P. Navrátil, and S. R. Stroberg for many useful discussions. This work was supported in part by JSPS KAKENHI Grant Number JP16J05707 and by the Program for Leading Graduate Schools, MEXT, Japan. This work was also supported in part by MEXT SPIRE and JICFuS (project IDs hp160211 and hp170230), and the CNS-RIKEN joint project for large-scale nuclear structure calculations.
Appendix A Decoupling equations
In this appendix, we briefly explain how to determine the correlation operators used in the UMOA Suzuki:1982 (). Owing to the definition of the unitary operator as shown in Eq. (8), appears only in the - and higher-body cluster terms and does not affect cluster terms lower than -body clusters (for instance, two- and higher many-body correlation operators do not show up in the one-body cluster terms of Eqs. (14) and (17).). Therefore, we can sequentially solve correlation operators in the order from the one- to -body cluster terms. In the following, we focus on the determination of the -body correlation operator , provided that the correlation operators with the rank lower than , , , , , are already obtained. The correlation operator is determined so that has no matrix elements between the and states. For this purpose, we define the operators and projecting onto the space of particles occupying the orbits below and above the Fermi level, respectively. Then, the decoupling condition between the target space and its complement can be described as
Eq. (51) can be rewritten as