Core momentum distribution in two-neutron halo nuclei

Core momentum distribution in two-neutron halo nuclei

L. A. Souza F. F. Bellotti M. T. Yamashita T. Frederico Lauro Tomio Instituto Tecnológico de Aeronáutica, DCTA, 12228-900, S. José dos Campos, Brazil. Department of Physics and Astronomy, Aarhus University, DK-8000 Aarhus C, Denmark. Instituto de Física Teórica, UNESP - Universidade Estadual Paulista, 01156-970, São Paulo, Brazil Centro de Ciências Naturais e Humanas, Universidade Federal do ABC, 09210-580, Santo André, Brazil.
July 14, 2019
Abstract

The core momentum distribution of a weakly-bound neutron-neutron-core exotic nucleus is computed within a renormalized zero-range three-body model, with interactions in the s-wave channel. The halo wave-function in momentum space is obtained by using as inputs the two-body scattering lengths and the two-neutron separation energy. The core momentum densities are computed for Li, Be C and C. The model describes the experimental data for Li, Be and to some extend C. The recoil momentum distribution of the C from the breakup of C nucleus is computed for different two-neutron separation energies, and from the comparison with recent experimental data the two-neutron separation energy is estimated in the range KeV. The recoil momentum distribution depends weakly on the neutron-C scattering length, while the matter radius is strongly sensitive to it. The expected universality of the momentum distribution width is verified by also considering excited states for the system.

keywords:
Binding energies, Faddeev equation, halo-nuclei, three-body system

, , , 111Corresponding author: tobias@ita.br and

1 Introduction

The core recoil momentum distribution of radioactive two-neutron halo nuclei close to the drip line, extracted from breakup reactions at few hundreds MeV/A, are expected to be quite useful in order to get insights on the underlying neutron-neutron-core structure of these exotic nuclei [1, 2]. This is particularly clear in the example of Li breakup in a carbon target at 800 MeV/A [1], where the momentum distribution is characterized by tahe sum of two distributions, a narrow one with MeV/c and a wide one with MeV/c, given that is the variance associated with a normal distribution. The narrow momentum distribution should be associated with a large configuration of the two neutrons forming a halo structure. In this case the breakup occurs when the two neutrons are found quite far from the core, corresponding to a weakly-bound three-body system in the nuclear scale. On the other hand, the wide momentum distribution is related to the inner part of the halo neutron orbits, close to the core region.

An interesting aspect of two-neutron halo states, associated with the narrow core momentum distribution, is that the halo constituents should have a high probability to be found in the classically forbidden region, outside the potential range. Therefore, the halo wave function should be quite insensitive to details of the interactions, once the model is adjusted by the best known two- and three-body low-energy observables. Therefore, one natural observable is the the two-neutron separation energy, , which represent the three-body binding. For the two-body subsystems neutron-neutron and neutron-core , the appropriate observables are the corresponding scattering lengths (or, respective, two-body energies). With these arguments, studies with schematic potentials, such as contact interactions, have been quite successful in describing low-energy three-body structures for large two-body scattering lengths (when the corresponding energies are close to zero). Actually, investigations on quantum three-body systems within this regime, in nuclear and atomic physics, became quite well known in view of recent experimental realizations in atomic laboratories of the long-time predicted Efimov effect [3], which corresponds to the increasing number of excited three-body states as one goes to the unitary limit (when one or both two-body scattering lengths are close to infinity). For recent reports, quoting the main experimental realizations of this effect, see Refs. [4, 5].

By considering a contact interaction, the corresponding wave-function is an eigenstate of the free Hamiltonian, except in the positions where the particles are right on the top of each other; and, therefore, the particles are in the classically forbidden region (see, e.g., [6]). Such theoretical approach applied to light-exotic nuclei close to the neutron drip-line, within a neutron-neutron-core () configuration, is described in detail in a recent review, in Ref. [7], where universal aspects of the properties of the weakly-bound systems are emphasized.

Our focus here is to present a theoretical investigation concerned to the experimental core recoil momentum distributions of the halo-nuclei Li [1], Be [8], C and [9], as obtained by the halo breakup on nuclear targets (see also Ref. [10]). The approach is the above described three-body model, which we found appropriate for the analysis of low-binding energy systems as these ones. In the particular cases of Li, Be and the carbon systems C and C, we consider that the neutron-neutron and the neutron-core interactions are dominated by wave states. The calculations of core momentum distributions are performed within a renormalized zero- range three-body model, with the halo nucleus described as two neutrons with an inert core ([7, 11]. The detailed expressions for the momentum distribution are given in [12], within an approach that requires as inputs one two-body () and one three-body ( ) observable, given that the other two-body observable is fixed to the well-known virtual-state energy of the system. Usually, within such approach it is appropriate to consider the corresponding two-body scattering lengths (positive, for bound, and negative for virtual state systems); with a three-body scale given by the two-neutron separation energy, . Therefore, in a more general description of low-energy three-body physics with two distinguished particles (), an appropriate universal scaling function is given (see e.g. [7]), where only three low-energy inpus are enough to determine any other relevant low-energy observable of the system.

Within our study on the momentum distributions of the core in halo nuclei the observable that we are concerned is the variance of the momentum distribution, given by (associated with the normal one), which is universally correlated to the two possible scattering lengths and . One obtains from the Full Width at Half Maximum (FWHM) of the momentum distribution, such that on can find that FWHM . Once this quantity is known experimentally, one can use the scaling function to estimate the value of or, eventually, to constraint some other poorly known low-energy observable, such as a subsystem energy, or scattering length. The natural units for in halo physics is MeV/c. As we are interested in scaling properties of observables, it is convenient to introduce the dimensionless ratio , where is the neutron mass. By taking as the mass unit, a scaling function can be defined, with a general form given by

(1)

where the and signs refer to the bound and virtual subsystem energies, respectively. The core mass number is . The corresponding energies, and , are positive defined quantities, with and being the respective two-body scattering lengths. In our specific case of the two-neutron halo nuclei the above scaling function (1) has fixed to the virtual state. In the next, our units are such that the Planck constant and the velocity of light are set to one. All masses are taken in units of .

For the momentum distribution width, the scaling function (1) is the limit cycle of the correlation function associated with as a function of , and , when the three-body ultraviolet (UV) cut-off is driven to infinite in the three-body integral equations, or equally the scattering lengths driven to zero with a fixed UV cut-off. Similar procedure is performed within a renormalized zero-range three-body model, in the subtracted integral equations, where the subtraction energy is fixed and the two-body scattering lengths are driven towards infinite. In practice, both procedures provides very close results, as shown in Ref. [13]. In the exact Efimov limit (), the width is a universal function of the mass number , which is associated to a limit cycle. Already in the first cycle it approaches the results of the renormalized zero-range three-body model (see e.g. [7]), namely given by the subtracted Skorniakov and Ter-Martirosian equations for mass imbalanced systems [14].

For the analysis of the core momentum distribution, we consider data for Li [1], Be [8] and [9] as the low-energy parameters, which are the inputs of our renormalized zero-range model. This procedure allows us to verify the utility of such “bare” formula (1), which does not include distortion effects from the scattering, to analyse the actual breakup data for those systems, taken at few-hundred MeV/A.

As an application of our model, we study in more detail the two neutron halo of the Borromean nuclei C, in an attempt to extract information of the halo properties, by using the correlation between observables expressed in Eq.(1), namely the width of the core recoil distribution as a function of and the energy of the wave virtual state of C. From the experimental point of view the two-neutron separation energy of C is not well constrained, with a value of 0.42 0.94 MeV given by systematics  [15] and from a mass measurement, it was found -0.14(46) MeV[16]. There is an indirect evidence that C could be bound by less than 70 keV [17]. Other independent information on the binding energy of this nucleus can be obtained from the matter radius. Tanaka and collaborators [18] extracted a root-mean-square (rms) matter radius of  fm from the analysis of the large reaction cross sections of C on liquid hydrogen target at 40A MeV, using a finite-range Glauber calculation under an optical-limit approximation. Furthermore, the two-valence neutrons occupy preferentially one orbital in their analysis. Such rms matter radius, taken together with the corresponding one of C (2.98(5) fm[19]), suggest a halo neutron orbit with rms radius of  fm in C, which is constraining the to be below 100 keV [20]. This value is consistent with results obtained from a shell-model approach [21] and results from effective field theory with contact interaction [22, 23]. The estimated C quantities should be compared with the fairly small value of keV for Li in the nuclear scale [24], and with the neutron-neutron () average separation distances in Li around 6-8 fm, which is obtained from the correlation function measured by the breakup cross-section on heavy nuclei [25, 26]. However, Riisager [2] pointed out that a comparison of experimental data obtained for the core recoil momentum distributions of Li [1] and [9] suggests similar neutron halo sizes for these nuclei, which could indicate an overestimation of the matter radius of this carbon isotope.

Our present work can give more insights in resolving the issue of the size of the two neutron halo in C. The constraints in the parameters associated with the C halo structure and two-neutron separation energy provided by the scaling formula for the width of the core recoil momentum distribution are discussed on the basis that corresponding data, fitted to three-body model calculations. The particular case of C is interesting considering that the corresponding observables are probably dominated by the tail of the three-body wave function in an ideal wave three-body model. That ideal structure was already considered in Ref. [27], within a Borromean C configuration for C, where all two-body subsystems, C and are not bound.

As it will be shown in the following, the recent experimental results for C and C [9] allow us, in principle, to constraint and the matter radius of C, even considering that the scattering length of the subsystem neutron-C is not well known. From the experimental analysis performed in Ref. [17], the associated wave virtual-state energy of C is found to be about MeV.

The present study on the constraint for are relying on the applicability of the renormalized three-body zero-range model and scaling function (1) derived for the width of the core recoil momentum distribution. In the case of C, this is obtained by fitting this distribution to the experimental breakup cross-section data given in Ref. [9]. For our estimative of is also essential that the scaling function given in (1) has a weak dependence of the ratio.

One of the sources of information on the sizes of unstable neutron-rich nuclei, is the correlation function obtained from Coulomb breakup experiments with neutron rich projectile on heavy nuclei [28, 25, 26]. The experimental results for the correlation function for Borromean nuclei Li and Be are found quite consistent with the corresponding computed quantities obtained within a subtracted renormalized zero-range model [29], unless an unexpected theoretical minimum before the correlation function approach unity for large relative momentum. Data from the experiments are showing a monodic decrease of the correlation function with momentum; however, the accessible data goes only up to the predicted minima region.

Next, we present the basic formalism. In section 3 we have the main results, followed by the section 4 where we summarize our conclusions.

2 Model formalism

In the following, we briefly sketch the formalism, based on the renormalized zero-range three-body model, leading to the core recoil momentum distribution formula, which is used in our data analysis of the halo nuclei systems Li, Be, C and C.

The renormalized zero-range model which we are considering to describe the halo wave-function has been explained in detail in the review [7]. In order to built the wave three-body wave function for the system, one needs to solve a coupled integral equation for the independent spectator functions and . Within the zero range model, a regularization is needed, which can be implemented with a cutoff momentum parameter, such as in Ref. [30], or by considering the subtraction procedure used in  [31], which we follow in the present approach. Therefore, the present subtractive regularization approach for the spectator functions is performed at a given energy scale , by the following coupled equations:

(2)

where

(3)
(4)

The above set of coupled equations can also be derived from a renormalized Hamiltonian as shown in [7], where the associated renormalization group properties are also discussed. The minus () sign refers to a bound state subsystem and the plus sign () to a virtual state subsystem. Therefore, within the perspective of a more general system, the following cases can be described by the above coupled integral equations: all-bound configuration, when there is no unbound subsystems; Borromean configuration, when all the subsystems are unbound; tango configuration [32, 33, 35], when we have two unbound and one bound subsystems; and samba configuration [31], when just one of the two-body subsystems is unbound. In the present case, as we are concerned with halo nuclei system, only samba and Borromean configurations are possible, once we take that is unbound with a virtual-state energy of about keV. This implies that only the sign is to be considered for in Eq. (3).

One can further simplify Eq. (2), for numerical purpose, by having an uncoupled integral equation for :

The corresponding wave three-body wave-function can be written in terms of the spectator functions and as:

(6)

where is the relative Jacobi momentum basis, with the relative momentum of the core to the center-of-mass of the system, and the relative momentum between the two neutrons. Note that, as we are going to present results corresponding to the limit cycle, namely, when all involved energies tends to zero with respect to the subtraction or regularization scale, we have dropped the regularization term in the denominator of the wave-function, which was introduced in Ref. [31]. The configuration space halo wave-function, which is given by the Fourier Transform of the momentum wave-function, is an eigenstate of the free Hamiltonian, except when two particles are at the same point, such that in our model the two halo-neutrons are always found in the classically forbidden region. This model can represent a real halo state as long as the neutrons have a large probability to be found outside of the potential range and of the core.

From the wave-function, given in momentum space by Eq. (6), we can define the core momentum distribution for the system as

(7)

with normalization such that . In the context of cold atoms the large momentum behaviour of the above momentum density has been studied in detail for three-bosons in  [34] and for mass imbalanced systems in [12]. The log-periodic solution of the spectator equations (2) in the ultraviolet limit, when , is the key property to derive asymptotic formulas for the one-body momentum densities. Furthermore, it was verified in [12] how the solutions of (2) approaches the log-periodic form for the higher Efimov excited states. In addition, it was shown that the density properties at low momentum behaviour are universal, namely, approach the limit-cycle already for the ground state with finite , and depend on the three-body binding energy and scattering lengths.

3 Results and discussion

The solution for the set of integral equations (2) provides the spectator functions and ultimately the momentum probability density (7). We start by showing results for , in order to study the limit-cycle for the core momentum distribution in the context of the two-neutron halo nuclei. To illustrate this limit we show in Fig. 1 the corresponding scaling function (1) for , in terms of the dimensionless ratio as a function of the core mass number. Results for the ground and two excited states in Fig. 1 show that the limit-cycle is universal and in practice found for the ground state. We compare with the experimental values of obtained for Li, MeV/c, coming from the halo breakup reaction Li +CLi + X at 800 MeV/A [1], and for Be, which has a FWHMMeV/c for the core recoil momentum distribution [8] and 1.337 MeV [15]. The flattening of the scaling function for large reaching an asymptotic value can be understood by inspecting the set of coupled equations (2) and the wave-function (6) by noticing that the limit can be performed, where all dependences on are cancelled out. One has to remind that even for the dependence of the core momentum distribution on the relative momentum just reflects the momentum distribution of the center of mass the two halo-neutrons in the nucleus. On the other hand, for , the momentum distribution tends be concentrated at small momentum as one can easily check that the relevant contribution to the integral equation for the spectator function comes from small momentum and . Naively, the light particle explores large distances, as the characteristic momentum is of the order of , and therefore for .

Figure 1: Scaling plot for the core recoil momentum distribution in the Efimov limit as a function of the core mass number . Experimental widths are from Refs. [1] and [8], for Li and Be, respectively.

The dependence of on the subsystems energies and is investigated by considering the results presented in Figs. 2 and 3, where we consider the Borromean configurations, in the cases of Li, Be and C, as well as the samba type configuration (bound subsystem), which is exemplified by the case of C. For and by changing from 0 to 143 keV, increases with respect to , as is seen when the values at the origin of these figures are compared to Fig. 1. It means that the halo shrinks as the virtual state energy increases in absolute value. This effect was found in [31], namely for a given the size of the halo shrinks when going from all-bound configuration to the Borromean one. This behaviour happens because the interaction becomes less attractive, such that to keep the three-body binding energy the state has to become smaller. This effect is also observed as the value of increases in for Li (left-frame) and Be (right-frame), as shown in Fig. 2. For the wave virtual state energy of Li of 50 keV, one has and MeV/c compared to the experimental value of MeV/c [1]. The experimental value of MeV/c from the FWHM of the momentum distribution of Be [8] is represented by the region delimited with the dashed lines in the right-frame of Fig. 2, and from that we could say roughly that wave virtual state of Be is less than 1 MeV, which is consistent with 0.2 MeV that is the known value (see e.g. [31]). We note that the dependence on is very mild and by changing it from 0 to a variation of of only 10% is found in our model, which puts a constraint in the error in the experimental ratio in order to be useful to extract information on the neutron-core virtual state energy.

Figure 2: Scaling plots for the core momentum distribution in Li (left-frame) and Be (right-frame) for the fixed 143 keV (virtual energy). The experimental 369 keV [24] and 1.337 MeV [15], for Li and Be, respectively. The dashed lines for Be represent the region delimited by the experimental value FWHMMeV/c [8].
Figure 3: Scaling plots for the core momentum distribution for C (left-frame) and C (right-frame), for a fixed keV (virtual-state energy). In the left frame, for C, we use 3.5 MeV [15]. In the right frame, for C, we use three values for : 100 keV (dashed line), 250 keV (dotted line) and 400 keV (solid line).

In Fig. 3, we show results for the scaling plots for the core momentum distribution in C (left-frame) and C (right-frame). In the left frame, the subsystem C forming the wave one neutron halo C is bound with energy 580 keV [15], where is the one neutron separation energy. Although, all halo low-energy scales are known for C, we allow variation of the ratio to illustrate how the width of the momentum distribution varies in the case of halo nuclei with bound subsystem. The width decreases as increases as the bound state energy becomes closer to the lowest scattering threshold, and consequently the neutron distance to core increases leading to the sudden drop of to zero, when goes to unity. In the right-frame of the figure, we present results for as a function of for C computed with different values of , 100 keV, 250 keV and 400 keV. We observe in the figure that while exhibits a strong dependence on with and kept constant, the variation of with the ratio for constant shows a quite weak sensitivity, as one could expect for the Borromean case. In that sense, as already recognized, the value of gives a good constraint for in this case.

Figure 4: Distributions of the recoil core in Li (left-frame) and C (right-frame) observed in the halo breakup reaction in a target compared to our calculations of the momentum distribution normalized to the data. The narrow distribution for Li is computed with 369 keV [24], wave virtual state energy of Li, =50 keV, and singlet virtual state, =143 keV. The results for the distribution with the computed narrow 22 MeV/c ( 21(3) MeV/c) are added to a wide one with 80 MeV/c. The calculations were performed for the experimental values from  [15] of 3.5 MeV for C, 580 keV for C. The experimental results for Li are extracted from [1] and for C from [9]. For Li the experiment detected the Li transverse momentum to the beam and for C the inclusive parallel momentum of C. The distribution for C was folded with the experimental resolution of MeV/c.
Figure 5: Left-frame: Distribution of the recoil core C obtained with the zero-range model compared to the experimental data from [9] for different inputs. For C the experiment detected the inclusive parallel momentum of C. Results for folded with the experimental resolution of MeV/c and added to a wide distribution with  MeV/c: solid-line (100,0), dashed-line (400,1) and dotted-line (100,1). Right-frame: Scaling plot for the core momentum width () in C (right frame) for given singlet virtual state energy (143 keV) and of 100 keV (dashed line), 250 keV (dotted line) and 400 keV (solid line).

After our discussion of the general scaling properties of the with of the momentum distribution, we show in Fig. 4 our calculations of the core recoil momentum distribution for Li (left-frame) and C (right-frame) compared to actual results from halo breakup experiments obtained reactions with carbon target at 800 MeV/A [1] and at 240 MeV/A [9], respectively. For Li, a wide distribution with 80 MeV/c is added to the computed narrow one, which has 22 MeV/c. We remark that all three inputs to compute the narrow distribution are fixed to known values of 369 keV [24], the wave virtual state energy of Li, =50 keV, and the singlet virtual state, =143 keV. The wide momentum distribution is beyond our model, which is more concerned on the halo neutrons. That contribution should be associated with inner part of the halo neutron orbits, close to the core region. In the comparison with the experimental data, the normalisations of the wide and narrow distributions are fitted to the data. After that, we find a fair reproduction of the experimental data as shown in the figure. This procedure confirms that our approach is a viable tool to extract information on the large two-neutron halo properties from the core momentum distribution.

The right-frame of Fig. 4 presents the core momentum distribution for C. The calculations were performed with 3.5 MeV and with C one-neutron separation energy equal to 580 keV [15]. The model is compared to data obtained from [9], after folding with the experimental resolution of MeV/c. We observe that a wide distribution is somewhat missing to fit the experimental results in this case.

The model results for the core recoil momentum distribution in C, with two-neutron separation energies of 100 and 400 KeV, is presented in the left-frame of Fig. 5, and compared to data obtained from [9]. The singlet virtual energy is fixed to 143 keV, with the virtual-state energy of C chosen as 0 and 1 MeV [17]. The narrow theoretical distribution is folded to the experimental resolution of MeV/c and added to a wide one with  MeV/c. The results presented in this figure illustrate the weak sensitivity of the core recoil momentum distribution to the variation of the virtual-state energy of C, which is taken between 0 and 1 MeV, as it was shown by the results with 100 keV. The difference between the distributions obtained with 100 and 400 keV, computed with MeV is not enough to discriminate in view of the experimental data error. The model sensitivity to the physical inputs, in the interesting case of C is further explored, in the right-frame of the figure, where the scaling plot for as a function of is shown for three values of . The weak sensitivity to the wave virtual state energy of C is seen and one could consider to obtain an upper limit to the experimental relative error in order to extract information on the C scattering length. However, a variation of the ratio between 0 and 9 gives 10% variation of ( is fixed), which is surmounted by a variation of about 50% in . Therefore, it is required an independent source of information to constrain the C scattering length, which we can find from the matter radius of C [18].

Figure 6: Root-mean-square (rms) matter radius of C given as a function of the two-neutron separation energy, computed with the singlet virtual-state energy fixed (143 keV), considering the virtual-state energy of C given by 1 MeV (left frame) and 0 MeV (right frame). The dashed lines represent the upper and lower limits for the experimental value  fm reported in [18].

To close our discussion of C, we computed the matter radius starting with the rms radius of the halo neutrons with respect to the center-of-mass, which is obtained from the configuration space wave-function, which is obtained by considering the Fourier transform of the corresponding momentum wave-function (6). For details on this procedure, see [31, 20]. The corresponding formula of the matter radius is given by . The C matter radius is 2.98(5) fm[19]. The plot of Fig. 6 shows the theoretical values of the rms matter radius of C as a function of for a fixed wave virtual state energies of the singlet pair (143 keV) and C (1 MeV [17] and 0) compared to data from [18]. In the figure, the limits for the extracted matter radius [18] are shown, and we can make some remarks analysing the consistence between the different available data and our model, considering that 100 keV keV: (i) for , one finds that 3.5 fm 4.5 fm; and, (ii) for MeV, we have 3.5 fm. Only if we obtain a region for close to 100 keV, consistent with rms matter radius of C within one standard deviation and in the lower bound of the radius, namely fm. The value of MeV for the virtual state of C and 100 keV is compatible with two standard deviation; from that, 3.5 fm. This combined analysis for C of the core recoil momentum distribution, with rms matter radius and virtual state energy of C, suggests that such virtual-state energy and matter radius are overestimated. Independent new data on the for C could help in clarifying the tension between data analysis with the present universal model.

4 Conclusions

In summary, by considering the renormalized zero-range model applied to the case of core recoil momentum distributions of Li and Be, we found a fair consistency with experimental data, just by using the known low-energy parameters. Relying on the fact that such simplified model gives already a valid description of the two-neutron -wave halo, we proceed with a combined analysis of recent experimental data on the core momentum distribution in C, which is given by Kobaiashi et al. [9], the corresponding rms matter radius and the C virtual state energy. Our conclusion is that, with the value of the two-neutron separation energy of C given in the interval from 100 to 400 keV, the rms matter radius of C will be within two standard deviations if the virtual state energy of C is close to 0. By considering the C with a virtual-state energy between 0 and 1 MeV, the matter rms radius should be between 3.5 and 4.5 fm. To reconcile a virtual-state energy with 1 MeV, a matter radius of 5.40.9 fm and 100 keV keV, the possibility is 100 keV and 1 MeV, implying that 4.5 fm. A refined analysis of the core momentum distribution, beyond the Serber model [36], is desirable, of course. However, the comparison of results obtained by the present model for Li and Be with corresponding data suggests small corrections to the distribution verified for C.

We thank partial support from the Brazilian agencies FAPESP, CNPq and CAPES.

References

  • [1] I. Tanihata, J. Phys. G 22 (1996) 157.
  • [2] K. Riisager, Phys. Scr. T152 (2013) 014001.
  • [3] V. Efimov, Phys. Lett. B 33 (1970) 563.
  • [4] V. Efimov, Few-Body Syst. 51 (2011) 79.
  • [5] F. Ferlaino, A. Zenesini, M. Berninger, B. Huang, H.-C. Nägerl, and R. Grimm, Few-Body Syst. 51 (2011) 113.
  • [6] T. Frederico, Few-Body Syst. 55 (2014) 651.
  • [7] T. Frederico, M. T. Yamashita, A. Delfino, and L. Tomio, Prog. Part. Nucl. Phys. 67 (2012) 939.
  • [8] M. Zahar, et al., Phys. Rev. C 48 (1993) R1484.
  • [9] N. Kobayashi et al., Phys. Rev. C 86 (2012) 054604.
  • [10] I. Tanihata, H. Savajols, and R. Kanungo, Prog. Part. Nucl. Phys. 68 (2013) 215.
  • [11] T. Frederico, L. Tomio, A. Delfino, M. R. Hadizadeh, M. T. Yamashita, Few-Body Syst. 51 (2011) 87.
  • [12] M. T. Yamashita, F. F. Bellotti, T. Frederico, D. V. Fedorov, A. S. Jensen, N. T. Zinner, Phys. Rev. A 87 (2013) 062702.
  • [13] M. T. Yamashita, T. Frederico, A. Delfino, L. Tomio, Phys. Rev. A 66 (2002) 052702.
  • [14] G. A. Skorniakov, K. A. Ter-Martirosian. Sov. Phys. JETP 4 (1957) 648.
  • [15] G. Audi, A. H. Wapstra, and C. Thibault, Nucl. Phys. A 729, 337 (2003).
  • [16] L. Gaudefroy et al., Phys. Rev. Lett. 109 (2012) 202503.
  • [17] S. Mosby et al., Nucl. Phys. A 909, 69-78 (2013)
  • [18] K. Tanaka et al., Phys. Rev. Lett. 104 (2010) 062701.
  • [19] A. Ozawa et al., Nucl. Phys. A 691 (2001) 599.
  • [20] M. T. Yamashita, R. M. de Carvalho, T. Frederico, L. Tomio, Phys. Lett. B 697 (2011) 90; Phys. Lett. B 715 (2012) 282.
  • [21] H. T. Fortune, R. Sherr, Phys. Rev. C 85 (2012) 027303.
  • [22] B. Acharya, C. Ji, D. R. Phillips, Phys. Lett. B 723 (2013) 196.
  • [23] B. Acharya, D. R. Phillips, arXiv:1508.02697 [nucl-th]. Contribution to the 21st Conference in Few-Body Problems in Physics.
  • [24] M. Smith et al., Phys. Rev. Lett. 101 (2008) 202501.
  • [25] F. M. Marqués, et al., Phys. Rev. C 64 (2001) 061301.
  • [26] M. Petrascu, et al., Nucl. Phys. A 738 (2004) 503.
  • [27] W. Horiuchi and Y. Suzuki, Phys. Rev. C 74 (2006) 034311.
  • [28] F. M. Marqués, et al. Phys. Lett. B 476 (2000) 219.
  • [29] M. T. Yamashita, T. Frederico, L. Tomio, Phys. Rev. C 72 (2005) 011601(R).
  • [30] A. E. A. Amorim, T. Frederico and L. Tomio, Phys. Rev. C 56 (1997) R2378.
  • [31] M. T. Yamashita, L. Tomio, T. Frederico, Nucl. Phys. A 735 (2004) 40.
  • [32] F. Robicheaux, Phys. Rev. A 60 (1999) 1706.
  • [33] A. S. Jensen, K. Riisager, D.V. Fedorov, E. Garrido, Rev. Mod. Phys. 76 (2004) 215.
  • [34] Y. Castin and F. Werner, Phys. Rev. A 83 (2011) 063614.
  • [35] N. T. Zinner, A. S. Jensen, J. Phys. G: Nucl. Part. Phys. 40 (2013) 053101.
  • [36] R. Serber, Phys. Rev. 72 (1947) 1008.
Comments 0
Request Comment
You are adding the first comment!
How to quickly get a good reply:
  • Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
  • Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
  • Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
""
The feedback must be of minimum 40 characters and the title a minimum of 5 characters
   
Add comment
Cancel
Loading ...
229583
This is a comment super asjknd jkasnjk adsnkj
Upvote
Downvote
""
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters
Submit
Cancel

You are asking your first question!
How to quickly get a good answer:
  • Keep your question short and to the point
  • Check for grammar or spelling errors.
  • Phrase it like a question
Test
Test description